text:
Types of Tea
Pu'er Tea
Purple Tea
Types of Tea Menu
Flowering tea, or blooming tea, consists of a ball made of tea leaves wrapped around one or more dried flowers. For tea drinkers, flowering tea is a way of infusing beauty itself into tea.
Two common names differentiate tea: Chinese tea and Indian tea. Chinese tea refers to tea made from the Camellia sinensis var. sinensis plant; Indian tea refers to tea made from the Camellia sinensis var. assamica plant. The way Camellia sinensis var. sinensis gets processed results in many different types of tea, two of which are white and green teas. Both of these types of tea are most often used in flowering tea.
The first section provides a summary of the general flavour of blooming tea, preparation, and its health benefits. The second section covers my thoughts and recommendations for different flowering teas. The third part discusses how flowering tea is made and the potential health benefits of flowers commonly included. The fourth and final section summarizes the key points discussed in this article.
Flavour, Preparation, and Health Benefits of Flowering Tea.
Flavour Profile Of Flowering Tea.
Flowering tea often has floral notes since flowers are used in its production. The most frequently used flowers are globe amaranth, chrysanthemum, jasmine, lily, rose, osmanthus and occasionally hibiscus. Depending on whether white or green tea is used in the production of a specific flowering tea, the flavour will be milder or more pronounced, respectively. Some tea experts find that, while often stunning, the taste of flowering teas may be less preferable than other teas.
How To Brew Flowering Tea.
First, place the tea ball into a glass teapot. Because the appeal of flowering tea is primarily the beauty of it unfolding, you should avoid opaque teapots. Since flowering tea is frequently made from green or white tea, use water that is between 140°F - 185°F and steep between three to five minutes. During this time, the bundle unfurls, imitating the blooming of a flower. Once fully expanded, the real flowers within the tea emerge as the centrepiece. When serving flowering tea, use glass cups to enhance the flavour.
Summary of Health Benefits of Flowering Tea.
The health benefits of flowering tea depend primarily on whether green or white tea was used in the ball, both of which contain potent antioxidants. Further health benefits depend on the specific flowers used in making the flowering tea.
Tea Recommendations and Personal Thoughts.
Mackenzie Bailey
Founder of The Tea Tribe
Flowering teas occupy a unique niche in the tea world. While there are some tasty flowering teas, this product is often less preferred by expert tea drinkers, as some find the taste to be less pleasing than other teas.
True Love Flower Tea and Two Dragons And A Pearl, both by Teavivre, are two flowering teas I enjoy.
On a per cup basis, flowering tea is more expensive than other options, which limits its appeal for regular consumption. However, flowering tea does offer a unique benefit: it is incredibly photogenic! Blooming tea can add a beautiful aesthetic to tea parties, or make a stunning shot for your Instagram feed.
A Comprehensive Discussion of Flowering Tea.
Most flowering tea is made in and imported from the Yunnan and Fujian provinces of China, where skilled tea artisans craft each ball of blooming tea by hand, manually binding tea leaves around flowers into a sphere. Sweet edible flowers are sewn together into the center of the ball and then flattened white or green tea leaves are sewn over the ball, forming the blooming tea's outer layer. Once built, the ball of flowering tea is dried.
Production of Flowering Tea.
"Our flowering tea is one of our best selling products! The beautiful appearance and taste of our blooming tea make our customers happy.
All our products get made with high-quality Maofeng Green Tea, Globe Amaranth, Marigold and Jasmine flowers. Then, each tea ball gets carefully handcrafted into shape. The process that goes into each tea ball is complex and requires a lot of time and patience.
TeaVivre sells twelve types of flower tea: each has a unique name with positive and symbolic meaning. "
Mary Bao,
Customer Service Manager, TeaVivre
Flowers Frequently Used And Their Health Benefits.
Flowers frequently used include globe amaranth, chrysanthemum, jasmine, lily, hibiscus, rose and osmanthus.
Globe Amaranth.
In traditional Chinese medicine, globe amaranth (Gomphrena globosa) is used to treat many respiratory conditions (Silva, 2012). Studies have found globe amaranth to be a powerful antioxidant (Roriz, 2017) (Roriz, 2014), and pairs synergistically with other plants, like lemongrass (Roriz, 2015).
Chrysanthemum.
Mums or chrysanths (Chrysanthemum) are primarily used to enhance the aroma of flowering tea. A recent study found that multiple types of chrysanthemum tea exhibited strong radical scavenging effects (Han, 2019), which are highly beneficial for health. One study found chrysanthemum had anti-inflammatory properties (Luyen, 2015), while another suggested that chrysanthemum may be helpful to those with type 2 diabetes (Bai, 2018).
Jasmine.
Jasmine (Jasminum) has a heavenly aroma and a long history of being used in tea production. In India, jasmine has been traditionally used to treat body pains, toothache, stomach aches and ulcers (Arun, 2015).
Chemical analysis of the flower shows that jasmine contains secoiridoids, terpenoids, flavonoids and tannins. Some research suggests secoiridoids protect blood lipids from oxidative stress (Celano, 2018), while terpenoids may reduce inflammation and pain (Gallily, 2018). Flavonoids are antioxidants, and some research suggests jasmine leaf extracts can benefit those with anxiety and epilepsy (Addae, 2017). Research into the impact tannins have on human health is mixed: some find it harmful, others positive (Chung, 1998).
Lily Flowers.
While being famed for their scent, the lily flower (Lilium) may also have some health benefits. Lilies have antioxidant, anti-inflammatory, and sedative capacities (Wang, 2015), and research also suggests that when consumed, lilies may help treat immune-related diseases (Pan, 2018).
Hibiscus.
The health benefits of hibiscus (Hibiscus rosa-Sinensis) is well documented. Hibiscus contains a significant amount of antioxidants; one study conducted on rats found hibiscus extract caused a 92% decrease in the harmful effects of free radicals (Tsai, 2002). Hibiscus is also known to lower systolic blood pressure (Mckay, 2009).
Rose.
Rose is a fragrant flower and is often used in flowering tea. Rose has anti-HIV, antibacterial, antidiabetic and antioxidant properties. It also can prevent coughs, induce sleep and has relaxant effects (Boskabady, 2011). Rose may depress the central nervous system somewhat (Nyeem, 2006), leading to a feeling of relaxation. Research has also established that rose positively impacts mood, and decreases anxiety and depression (Rakhshandah, 2004) (Rakhshandah, 2006) (Boskabady, 2011).
Rose can also have beneficial effects on brain function. One study found rose promotes neuron growth in the brain and may help protect against Alzheimer's disease (Awale, 2011). Multiple studies have documented a positive impact of rose tea on seizures and epilepsy (Kheirabadi, 2011; Moghimi, 2008; Ashrafzadeh, 2007).
Osmanthus.
Osmanthus is a genus that includes 30 flowering plant species. Flowering tea uses many of these flowers, with sweet osmanthus (Osmanthus fragrans) being particularly common. Traditional Chinese medicine credits tea made with osmanthus for improving complexion and helping the body get rid of excess nitric oxide, which is linked to cancer and diabetes (Wikipedia, 2019). Some research supports osmanthus's standing in traditional Chinese medicine as an anticancer agent, and one study found Osmanthus matsumuranus could be a chemopreventive agent (Jin, 2015).
Flowering (or blooming) tea is often made with either white or green tea. When preparing flowering tea, the water should be between 140°F - 185°F and the tea should steep for three minutes or longer, based on taste preference.
True to its namesake, at least one flower gets used when making the tea. Flowers are placed, by hand, at the heart of a tea ball through a painstaking process. When a flowering tea ball is put into water, it unfurls in a process reminiscent of a blooming flower.
The health benefits of flowering tea depend on the type of tea used, as well as the kind of flower included in each specific ball.
Flowering tea may not always live up to what tea drinkers expect from the taste, but it has an aesthetic appeal that no other tea can match.
In the comments below, please share your favourite flowering tea.
Addae, J. I., Pingal, R., Walkins, K., Cruickshank, R., Youssef, F. F., & Nayak, S. B. (2017). Effects of Jasminum multiflorum leaf extract on rodent models of epilepsy, motor coordination and anxiety. Epilepsy Research, 131, 58–63. http://doi.org/10.1016/j.eplepsyres.2017.02.012
Arun, M., Satish, S., & Anima, P. (2015). Phytopharmacological Profile of Jasminum grandiflorum Linn. (Oleaceae). Chinese Journal of Integrative Medicine, 22(4), 311–320. http://doi.org/10.1007/s11655-015-2051-3
Ashrafzadeh, F., Rakhshandah, H., & Mahmoudi, E. (2007). Rosa damascena oil: an adjunctive therapy for pediatric refractory seizer. Iranian Journal of Child Neurology, 1, 13–17. Retrieved from http://journals.sbmu.ac.ir/ijcn/article/view/595
Awale, S., Tohda, C., Tezuka, Y., Miyazaki, M., & Kadota, S. (2011). Retracted: Protective Effects of Rosa damascena and Its Active Constituent on Aβ(25–35)-Induced Neuritic Atrophy. Evidence-Based Complementary and Alternative Medicine, 2011. Retrieved from https://www.ncbi.nlm.nih.gov/pubmed/19789212
Bai, Y., Li, K., Shao, J., Luo, Q., & Jin, L. (2018). Flos Chrysanthemi Indici extract improves a high-sucrose diet-induced metabolic disorder in Drosophila. Experimental and Therapeutic Medicine, 16(3), 2564–2572. http://doi.org/10.3892/etm.2018.6470
Boskabady, M. H., Shafei, M. N., Saberi, Z., & Amini, S. (2011). Pharmacological Effects of Rosa Damascena. Iranian Journal of Basic Medical Sciences, 14(4), 295–307. Retrieved from https://www.ncbi.nlm.nih.gov/pmc/articles/PMC3586833/
Celano, R., Piccinelli, A. L., Pugliese, A., Carabetta, S., Sanzo, R., Rastrelli, L., & Russo, M. (2018). Insights into the Analysis of Phenolic Secoiridoids in Extra Virgin Olive Oil. Journal of Agricultural and Food Chemistry, 66(24), 6053–6063. http://doi.org/10.1021/acs.jafc.8b01751.
Chung, K. T., Wong, T. Y., Wei, C. I., Huang, Y. W., & Lin, Y. (1998). Tannins and human health: a review. Critical Reviews in Food Science and Nutrition, 38(8), 421–464. http://doi.org/10.1080/10408699891274273
Gallily, R., Yekhtin, Z., & Hanuš, L. O. (2018). The Anti-Inflammatory Properties of Terpenoids from Cannabis. Cannabis and Cannabinoid Research, 3(1), 282–290. http://doi.org/10.1089/can.2018.0014
Han, A.-R., Nam, B., Kim, B.-R., Lee, K.-C., Song, B.-S., Kim, S., … Jin, C. (2019). Phytochemical Composition and Antioxidant Activities of Two Different Color Chrysanthemum Flower Teas. Molecules, 24(2), 329. http://doi.org/10.3390/molecules24020329
Jin, S., Park, H.-J., Oh, Y. N., Kwon, H. J., Kim, J.-H., Choi, Y. H., & Kim, B. W. (2015). Anti-cancer Activity of Osmanthus matsumuranus Extract by Inducing G2/M Arrest and Apoptosis in Human Hepatocellular Carcinoma Hep G2 Cells. Journal of Cancer Prevention, 20(4), 241–249. http://doi.org/10.15430/jcp.2015.20.4.241
Kheirabadi, M., Moghimi, A., Rakhshande, H., & Behnam Rassouli, M. (2008). Evaluation of the Anticonvulsant Activities of Rosa damascena on the PTZ Induced Seizures in Wistar Rats. Journal of Biological Sciences, 8(2), 426–430. http://doi.org/10.3923/jbs.2008.426.430
Luyen, B. T., Tai, B. H., Thao, N. P., Cha, J. Y., Lee, H. Y., Lee, Y. M., & Kim, Y. H. (2015). Anti-inflammatory components of Chrysanthemum indicum flowers. Bioorganic & Medicinal Chemistry Letters, 25(2), 266–269. http://doi.org/10.1016/j.bmcl.2014.11.054
Mckay, D. L., Chen, C.-Y. O., Saltzman, E., & Blumberg, J. B. (2009). Hibiscus Sabdariffa L. Tea (Tisane) Lowers Blood Pressure in Prehypertensive and Mildly Hypertensive Adults. The Journal of Nutrition, 140(2), 298–303. http://doi.org/10.3945/jn.109.115097
Moghimi, A., Ramezani, R., Rakhshandeh, H., Ejtehadi, H., & Kheirabadi, M. (2008). The Effect of Rosa damascena Essential Oil on the Amygdala Electrical Kindling Seizures in Rat. Pakistan Journal of Biological Sciences, 11(5), 746–751. http://doi.org/10.3923/pjbs.2008.746.751
Nyeem, M. A. B., Alam, M. A., Awal, M. A., Mostofa, M., Uddin, M., Islam, S. J. N., & Rouf, R. (2006). CNS Depressant Effect of the Crude Ethanolic Extract of the Flowering Tops of Rosa Damascena. . Iranian Journal of Pharmacology & Therapeutics , 5, 171–174. Retrieved from https://www.researchgate.net/profile/Shaikh_Uddin/publication/43561261_CNS_Depressant_Effect_of_the_Crude_Ethanolic_Extract_of_the_Flowering_Tops_of_Rosa_Damascena/links/09e4150a2946854dc1000000/CNS-Depressant-Effect-of-the-Crude-Ethanolic-Extract-of-the-Flowering-Tops-of-Rosa-Damascena.pdf
Pan, G., Xie, Z., Huang, S., Tai, Y., Cai, Q., Jiang, W., … Yuan, Y. (2018). Corrigendum to "Immune-enhancing effects of polysaccharides extracted from Lilium lancifolium Thunb" [Int. Immunopharmacol. 52 (2017) 119–126]. International Immunopharmacology, 58, 119–126. http://doi.org/10.1016/j.intimp.2017.12.033
Rakhshandah, H., Hosseini, M., & Dolati, K. (2004). Hypnotic effect of Rosa damascena in Mice. Ranian Journal of Pharmaceutical Research, 3, 181–185. http://doi.org/10.22037/IJPR.2010.598
Rakhshandah, H., & Hosseini, M. (2006). Potentiation of pentobarbital hypnosis by Rosa damascena in mice.Indian Journal of Experimental Biology, 44, 910–912. Retrieved from https://www.ncbi.nlm.nih.gov/pubmed/17205713
Roriz, C. L., Barros, L., Carvalho, A. M., Santos-Buelga, C., & Ferreira, I. C. (2014). Pterospartum tridentatum, Gomphrena globosa and Cymbopogon citratus: A phytochemical study focused on antioxidant compounds. Food Research International, 62, 684–693. http://doi.org/10.1016/j.foodres.2014.04.036
Roriz, C. L., Barros, L., Carvalho, A. M., Santos-Buelga, C., & Ferreira, I. C. (2015). Scientific validation of synergistic antioxidant effects in commercialised mixtures of Cymbopogon citratus and Pterospartum tridentatum or Gomphrena globosa for infusions preparation. Food Chemistry, 185, 16–24. http://doi.org/10.1016/j.foodchem.2015.03.136
Roriz, C. L., Barros, L., Prieto, M., Morales, P., & Ferreira, I. C. (2017). Floral parts of Gomphrena globosa L. as a novel alternative source of betacyanins: Optimization of the extraction using response surface methodology. Food Chemistry, 229, 223–234. http://doi.org/10.1016/j.foodchem.2017.02.073
Silva, L. R., Valentão, P., Faria, J., Ferreres, F., Sousa, C., Gil-Izquierdo, A., … Andrade, P. B. (2012). Phytochemical investigations and biological potential screening with cellular and non-cellular models of globe amaranth (Gomphrena globosal.) inflorescences. Food Chemistry, 135(2), 756–763. http://doi.org/10.1016/j.foodchem.2012.05.015
Tsai, P.-J., Mcintosh, J., Pearce, P., Camden, B., & Jordan, B. R. (2002). Anthocyanin and antioxidant capacity in Roselle (Hibiscus Sabdariffa L.) extract. Food Research International, 35(4), 351–356. http://doi.org/10.1016/s0963-9969(01)00129-6
Wang, T., Huang, H., Zhang, Y., Li, X., Li, H., Jiang, Q., & Gao, W. (2015). Role of Effective Composition on Antioxidant, Anti-inflammatory, Sedative-Hypnotic Capacities of 6 Common EdibleLiliumVarieties. Journal of Food Science, 80(4), 857–868. http://doi.org/10.1111/1750-3841.12787
Wikipedia. (2019, May 6). Osmanthus. Retrieved July 30, 2019, from https://en.wikipedia.org/wiki/Osmanthus
© 2022, The Tea Tribe Powered by Shopify


Dr. Roos received her medical degree from Wake Forest University School of Medicine in Winston-Salem, NC. She completed her internship and residency at Self Regional Hospital in Greenwood, SC. Dr. Roos is board certified in Family Medicine.


Lady Dream Granite Stone enhances the beauty of the place, where it is used. We are counted among the top companies, which are engaged in manufacturing and supplying Lady Dream Granite Stone. The cutting and finishing of our Lady Dream Granite Stone is done under the supervision of industry experts. Thus, our Lady Dream Granite Stone is the perfect option on which buyers can easily rely.


Featuring free WiFi and a restaurant, Hotel Verde Mare offers pet-friendly accommodation in Santarcangelo di Romagna. Guests can enjoy the on-site restaurant. Free private parking is available on site. All rooms include a TV.


All Brown Haven Home plans include luxury finishes and superior products. The RiverStone single-family home plan is 3,564 square feet, has 4 bedrooms, 2.5 bathrooms, and 2 garage spaces. Starting from $277,268, the RiverStone home can be built "On Your Lot" in Ellijay, Georgia. Other nearby locations you can build a new RiverStone home include Gilmer County, Chatsworth in Murray County, and Pickens County, Georgia. In all, we build our award-winning custom homes in twenty-one Georgia counties. Similar custom homes in Ellijay you may love include the 3,745 square foot MeadowView plan, the MistyRidge, a 3.5-bath home, and the 4 bedroom MountainRidge custom home.


text:
California's Drought May Be Worst in a Millennium
The record in trees suggests this drought is the worst to hit the Golden State in as much as 1,200 years
By Niina Heikkinen, ClimateWire on December 5, 2014
When Daniel Griffin first heard media reports earlier in the fall that California's drought was the worst in the past few centuries, he didn't quite buy it.
Griffin, an assistant professor in the Department of Geography, Environment and Society at the University of Minnesota, had a decade of experience studying paleoclimate and environmental science using tree-ring data. From his research on blue oak trees, he knew that periods without a lot of precipitation weren't that uncommon in the state's history.
"I was kind of skeptical that this year would be different," he said.
Still, Griffin was curious to see if the blue oaks he was studying could provide clues about the state's three-year drought. The trees are particularly sensitive to changes in water availability, and their rings clearly showed changes in moisture levels over the trees' lifetime.
"When it's very dry, they grow very slow; when it's a wet year, they grow like gangbusters," he said.
The trees are long-lived. They can be up to 500 years old, and deadwood like stumps can stay in the ground for around 700 years, providing an extended record of water availability over centuries. They are also native to Southern and Central California, where the drought has been the most severe.
Griffin, along with Kevin Anchukaitis, an assistant scientist at Woods Hole Oceanographic Institution, began taking pencil-thin tree-ring samples from trees to see how they were responding to the drought compared to previous years.
The researchers compared their tree-ring data with National Oceanic and Atmospheric Administration precipitation measurements from between 1920 and 2014, and used that information to reconstruct precipitation history before rain gauge measurements began.
To compare the present drought to the magnitude of past events, the researchers used the Palmer Drought Severity Index, a proxy for soil moisture that includes temperature effects, from the North American Drought Atlas, which was developed by the Lamont-Doherty Earth Observatory at Columbia University and extends back 1,200 years.
Their analysis showed that a number of other droughts in California's history had less precipitation than the one the state is currently experiencing. However, the most recent drought stood out because of how exceptionally hot it was compared to other droughts over the past 1,200 years.
Even when they accounted for errors associated with combining the different data sets, they saw that "what's really different is the record high temperatures," Griffin said.
"That kind of knocked my socks off, I wasn't expecting that result," he said.
The "hot drought" was worse because the heat drew more moisture from the soil into the atmosphere, according to Griffin. For every 1 degree Celsius increase in air temperature, the atmosphere's capacity to retain moisture increases by 7 percent, as defined by the Clausius-Clapeyron equation.
A record that may not last for long
"Low precipitation is compounded by record high temperatures to create extreme drought," said Griffin.
Griffin and Anchukaitis published their findings in Geophysical Research Letters.
"This study really established how exceptional and severe this last drought was even in the last thousand years," said Benjamin Cook, a climate scientist at NASA's Goddard Institute for Space Studies who studies the drought on the West Coast. He was not involved in the study.
According to Cook, the modest declines in precipitation levels have not been enough to explain why the drought in California has been so bad. The study teased out how precipitation and temperature interacted to make dry conditions worse.
"The conclusion that I think is the most compelling is that warming from anthropogenic greenhouse gas emissions really made the drought more severe than it would have been," Cook said. "California is on track for the warmest year on their record."
The findings also raise concerns about what California could experience in the future, as well as how the state should plan to conserve its limited groundwater resources, said Park Williams, a professor at the Lamont-Doherty Earth Observatory.
"Regardless of how much of this year's heat was man-made or natural in origin, 2014 serves as an important reminder that heat can seriously exacerbate drought events," wrote Williams in an email. "If temperatures continue rising, we should expect record-breaking drought years to become increasingly common."
Reprinted from Climatewire with permission from Environment & Energy Publishing, LLC. www.eenews.net, 202-628-6500
Recent Articles by Niina Heikkinen
Clean Power Plan Replacement Could Lead to Increased Emissions
As Climate Scientists Speak Out, Sexist Attacks Are on the Rise
To Kill Climate Rule, EPA Proposes Redefining the Dangers of Soot
Recent Articles by ClimateWire
Some Disaster Prevention Spending Reaps Higher Rewards
Climate Preparation Report Released by Panel Previously Disbanded by Trump
Greenland Has Yet Another Methane Leak

redpajama_set_name: RedPajamaCommonCrawl


Improved System Performance and Dependability - Industrial Resource Group, LLC.
The system malfunctions due to inherent design were eliminated.
System downtime related to power unit failure was reduced to ZERO.


text:
\section{Introduction}

In many-body systems described by classical mechanics the presence of an ordered phase is connected to the spontaneous breaking of symmetries
associated with local order parameters. A system consisting of classical spins, for instance, may admit a ground
state having all spins oriented along a given direction. Such ground states simultaneously break the spin-rotation and the time-reversal symmetry
witnessed by a non-vanishing magnetic moment.

Considering quantum systems, in contrast, one finds also different phases connected to some physical quantity but not necessarily to the magnetic
moment. The paradigmatic example is a translation invariant spin-$\frac{1}{2}$ chain for which the ground states correspond to the so called valence
bond states, i.e. states build up by tensor products of maximally entangled bipartite states~\cite{A1973,A1987}. In such systems neither the
spin-rotation nor the time-reversal symmetry is broken, nevertheless, it is possible to define order parameters characterizing the phases.
Typically nematic phases occur if at least one symmetry of the Hamiltonian is broken which are phases with long range ordering, i.e. defined by
order parameters on a finite set of sides. Other examples intensively discussed are topological order phases~\cite{W1990,KW2009} that, for instance,
are associated with the robustness of ground state degeneracies~\cite{WN1990}, are quantized non-Abelian geometric phases~\cite{W1990} or possess
patterns due to long-range quantum entanglement~\cite{CGW2010}.

Frustration occurs for systems with competing interactions or non-trivial geometries and can be related to quantum entanglement~\cite{GHI2014}.
Non-trivial spin orders are usually found if an interplay between frustration and quantum fluctuations is at work resulting in chiral, nematic or
general multipolar phases. In contrast to topological phases, even in the case of a vanishing magnetic moment the spin-rotation symmetry is
broken~\cite{AG1984,LMM2011}. These phases are also interesting from the point of applications. The topological ordered phases play
a fundamental role in the spin liquids~\cite{IHM2011,ZGV2011} and in non-Abelian fractional Hall systems~\cite{LH2008} and are
predicted to play a key role in the future development of fault-tolerant quantum computers~\cite{K2003}. The nematic order is usually found in
materials commercially used in the liquid crystal technology~\cite{TGC2010} such as LCDs (liquid crystal display).

Non-trivial ordered spins appear usually for higher dimensional systems (lattices) or sites with more than two degrees of freedom
(spins higher than $\frac{1}{2}$). Exceptions are the frustrated one dimensional ferromagnetic spin-$\frac{1}{2}$ chain in
an external magnetic field having a nematic ordered phase~\cite{C1991,HHV2006} and the one dimensional cluster-Ising model exhibiting a symmetry
protected topological ordered phase~\cite{SAFFFPV2011,MH2012,GH2014}.

In general, mathematical tools to handle such systems are rare and only few very specific Hamiltonians have been found to be analytically solvable.
The present paper introduces a huge class of analytically solvable one dimensional models with two degrees of freedoms (spin-$\frac{1}{2}$)
exhibiting both topologically and nematic ordered phases, which we dub $n$-cluster-Ising models. The index $n=1,2,\dots$ refers to the presence of
an $n+2$-body interaction, a cluster size of $n+2$. The physical systems under investigation are characterized by two competing interactions, a
two-body Ising interaction along the $y$-axis and an $n+2$-body interaction along the $x$-axis and the $z$-axis. The Hamiltonian of the family of
models can be written as
 \begin{equation}
  \label{Hamiltonian}
\!\!\! H^{(n)}\!\!=\!\!J\!\!\left(\!\sin(\phi)\!  \sum_{j} \!\sigma_{j}^y \sigma_{j+1}^y \!-\!\cos(\phi)\! \sum_{j}\! \sigma_{j}^x O^z_{j,n} \sigma_{j+n+1}^x
 \! \right)
 \end{equation}
where $J$ has the dimension of an energy (which we set equal to one in the computation) and $O^z_{j,n}$ stands for
\begin{equation}
\label{Oz_operator}
 O^z_{j,n} = \bigotimes_{k=1}^{n} \sigma_{j+k}^z \; .
\end{equation}
Via the parameter $\phi$ the relative weight of the two interactions is controlled: When $\phi$ approaches $0$ the system is dominated
by the multi-body interaction whereas when $\phi$ tends to $\pi/2$ the system is dominated by the (anti-ferromagnetic) Ising interaction.

We show that this family of models can be analytically solved (Sec.~\ref{Solution}) and how the spin correlation function can be obtained
(Sec.~\ref{Spincorrelation}). We prove that there is a quantum critical point at $\phi_c=\pi/4$  separating the cluster phase from the Ising phase.
This corresponds to the case when both interactions have equal weights. This critical point $\phi_c$, surprisingly, does not depend on the
$n+2$-body interaction, hence, it does not dependon the cluster size. In strong contrast to the relevant ordering in the cluster phase that depends strongly on $n$:
In case of odd $n$ a symmetry protected topologically ordered phase is present, whereas for even $n$ a nematic phase is present. In both cases we
determine the order parameter (string order parameter for the topological ordered phase and block order parameter for the nematic phase) as
well as the order parameter of the Ising phase (Sec.~\ref{Orderparameters}).

In the next step we study the various entanglement properties of the family of models (Sec.~\ref{Entanglementproperties}). The first observation is
that for any $n$ and $\phi$ -- as proven for the standard cluster-Ising model ($n=1$) in Ref.~\cite{GH2014} -- there is no bipartite entanglement.
Picking out any two spins the state is separable. Indeed, we find that this family of Hamiltonians lead to ground states that possess
\textit{genuine} $k=n+2$-partite entanglement between any contiguous spins and any $k<n+2$-partite entanglement vanishes. The symmetries in the
state space of the ground states force the reduced state of any $n+2$ adjacent spins into a so-called $X$-form~\cite{YE2007}, i.e. by applying
certain local unitary operators the reduced density matrix has only non-zero entries on the two diagonals. Due to this form we can exactly
evaluate a measure for genuine multipartite entanglement~\cite{HH2008,MCCSGH2011,HHBE2012}, i.e. quantify the entanglement content. So far, long
range multipartite entanglement close to a phase transition has been studied in terms of entanglement witnesses, e.g. for the $XXZ$ spin
chain~\cite{SRPCS2014} or for the $XY$ model~\cite{GH2013,Discord2014,CRGB2013}. Having this strong tool at hand, a measure of genuine multipartite
entanglement, we find that non-zero \textit{genuine} multipartite entanglement is only non-zero in the Ising phase $\phi>\phi_c$ (except $n=1$),
thus exhibiting a fortunate behaviour for applications such as utilizing these quantum systems for quantum algorithms.

The block entanglement properties are studied with focus around the quantum phase transition. Via the relation between conformal field
theory~\cite{HLW1994} and the divergence of the block entanglement at the quantum phase transition we are able to evaluate the central charges of
the models that turns out to depend on $n$.

Last but not least we conclude (Sec.~\ref{Conclusions}) by discussing the interplay between the characterization of the many-body systems by ordered
parameters and by symmetries in the Hilbert-Schmidt space of the ground states revealing the entanglement properties.

\section{Solution of the models}
\label{Solution}

In this section we present how to compute analytically the ground states of the models under investigation. The idea is to map the Hamiltonian,
Eq.~(\ref{Hamiltonian}), of spin-$\frac{1}{2}$ particles into non-interacting fermions moving freely along the chain only obeying Pauli's exclusion
principle. This method works even for the case in which the length of the system diverges~\cite{LSM1961,BM1971}. Having finally computed the energy
density function we find a phase transition that is further analysed in Sec.~\ref{Orderparameters}.

The mapping of a spin model to a fermionic one is obtained by applying the Jordan-Wigner transformation~\cite{JW1928}. Providing the correct
anti-commutation rules in the Jordan-Wigner transformation one associates the local spin operators with non-local fermionic operators
\begin{eqnarray}
\label{JWT}
 c_j = \bigotimes_{k=1}^{j-1}\left( \sigma^z_k \right) \sigma_j^- \;, \;\; \;& & \; \; \;
 c_j^\dagger = \bigotimes_{k=1}^{j-1} \left( \sigma^z_k \right) \sigma_j^+ \; ,
\end{eqnarray}
where $\sigma^\pm$ are the respective ladder operators. Herewith the Hamiltonian in Eq.~(\ref{Hamiltonian}) becomes
\begin{eqnarray}\label{Hamiltonian2}
  H^{(n)}\!\!&\!=\!&\! J\! \sin(\phi)  \! \sum_{j}\! \left( \! c_{j}^\dagger c_{j+1}^\dagger - c_{j}^\dagger c_{j+1}  + c_{j} c_{j+1}^\dagger - c_{j} c_{j+1}
  \right) \nonumber \\
  &\!+\!&\!J\!\cos(\phi) \sum_{j}\left( c_{j}^\dagger c_{j+n+1}
  - c_{j} c_{j+n+1}^\dagger\right.\nonumber\\
  && \;\;\;\;\;\;\;\;\;\;\;\;\;\;\;\;\;\;\;\; \left.+ c_{j}^\dagger c_{j+n+1}^\dagger - c_{j} c_{j+n+1}\right)
  \end{eqnarray}
One notes that herewith the cluster interaction is reduced from a $n+2$ interaction to a two-body interaction
between sites at distance $n+1$. After having reduced the problem to an effective two-body one the model can be diagonalized via the Fourier
transforms of the fermionic operators, i.e.
\begin{eqnarray}
\label{FT1}
 b_k & = & \frac{1}{\sqrt{N}} \sum_{j} c_k\; e^{-i\,kj}\; , \nonumber \\
 b_k^\dagger & = & \frac{1}{\sqrt{N}} \sum_{j} c_k^\dagger\; e^{i\,kj} \; ,
\end{eqnarray}
where the wave number $k$ is equal to $k=2 \pi l/N$ and $l$ runs from $-N/2$ to $N/2$ and $N$ is the total number of spins (sites) in the chain.
The Hamiltonian transforms to
\begin{eqnarray}
  \label{Hamiltonian3}
 H^{(n)} & = & \sum_{k>0} h_{k}^{(n)}
 \end{eqnarray}
 with
 \begin{eqnarray}
 h_{k}^{(n)}& =& 2\,i\, \delta_{k,n}\;  \left( b_{k}^\dagger b_{-k}^\dagger- b_{-k} b_{k}\right) \nonumber\\
 &&+
 2\, \varepsilon_{k,n}\; \left( b_{k}^\dagger b_{k}+ b_{-k}^\dagger b_{-k}-1 \right) \; , \nonumber
\end{eqnarray}
where the parameters $\delta_{k,n}$ and $\varepsilon_{k,n}$ are respectively given by
\begin{eqnarray}
  \label{deltaepsilon}
 \delta_{k,n}& = & J\;\left(\sin\left((n+1)k\right) \cos\phi+ \sin(k) \sin\phi\right)\;, \nonumber \\
 \varepsilon_{k,n} & = &  J\;\left(\cos\left((n+1)k\right) \cos\phi- \cos(k) \sin\phi\right)\; .
\end{eqnarray}
Via these transformations we re-wrote the Hamiltonian under investigation into the sum of non-interacting terms $h_{k}^{(n)}$, each one of them
acting only on fermionic states with wave number equal to $k$ or $-k$.  Each  $h_{k}^{(n)}$ corresponds to a four level system that can be
expressed in an occupation number basis by  $|1_k,1_{-k}\rangle$, $|0_k,0_{-k}\rangle$, $|1_k,0_{-k}\rangle$, $|0_k,1_{-k}\rangle$ and is,
explicitly, represented by the following matrix
\begin{equation}
 \label{Hamiltoniank}
h_{k}^{(n)}=\left(
\begin{array}{cccc}
2\; \varepsilon_{k,n} & +2\, i\; \delta_{k,n} & 0 & 0 \\
- 2\, i\; \delta_{k,n} & - 2\; \varepsilon_{k,n} & 0 & 0 \\
 0 & 0 & 0 & 0 \\
 0 & 0 & 0 & 0
\end{array}
\right) \; ,
\end{equation}
which ground state energy computes to
\begin{equation}
\label{Ek0}
 \!\!\!E_{k}^{(n)}\!\!=\!- 2\! \sqrt{\!\varepsilon_{k,n}^2\!+\!\delta_{k,n}^2}\!=\!- 2J\! \sqrt{\!1\!-\!\cos((n\!+\!2)k)\! \sin(2\phi)} \!\;.
\end{equation}
The associated ground state $|\psi_k^{(n)}\rangle$ is a superposition of $|1_k,1_{-k}\rangle$ and $|0_k,0_{-k}\rangle$
\begin{equation}
|\psi_{k}^{(n)}\rangle=\alpha_{k,n}\; |1_k,1_{-k}\rangle +\beta_{k,n}\; |0_k,0_{-k}\rangle
\end{equation}
with
\begin{eqnarray}
 \label{alphakbetak}
 \alpha_{k,n} &=& i \frac{\varepsilon_{k,n} +E_{k}^{(n)}}{\sqrt{\delta_{k,n}^2+(\varepsilon_{k,n}
 +E_{k}^{(n)})^2}} \; ,
 \nonumber \\
 \beta_{k,n} &=&  \frac{\delta_{k,n}}{\sqrt{\delta_{k,n}^2+(\varepsilon_{k,n}+ E_{k}^{(n)})^2}} \; .
\end{eqnarray}
Since the Hamiltonian is the sum of the non-interacting terms $h_{k}^{(n)}$, each one of them is acting on a different Hilbert space,
and the ground state of the total Hamiltonian is consequently a tensor product of all $|\psi_{k}^{(n)}\rangle$
\begin{equation}
 |\psi^{(n)}\rangle=\bigotimes_{k} |\psi_{k}^{(n)}\rangle\;.
\end{equation}
The associated energy density $E_{n,\phi}$ is the sum $E_k^{(n)}$ divided by the total number of the spins $N$. In the thermodynamic
limit the energy density becomes
\begin{equation}
 \label{E0}
E_{n,\phi}=-\frac{2J}{\pi} \int_0^\pi  \sqrt{1-\cos((n+2)k) \sin(2\phi)} dk \;.
\end{equation}

\begin{figure}
\includegraphics[width=0.49\textwidth]{newfig1.eps}
\caption{(Color online) The graphes show the second derivative of the energy density of the ground state $E_{n,\phi}$ as a function of $\phi$ for
different cluster sizes $n+2$. The divergence is independent of $n$ at the critical value $\phi_c=\frac{\pi}{4}$ and corresponds to a vanishing
energy gap between the ground state and the first excited state.}
\label{secondderivativeenergy}
\end{figure}

According to the general theory of continuous phase transitions at zero temperature~\cite{S2011} the presence of a quantum critical point is
signaled by the divergence of the second derivative of the energy density with respect to the Hamiltonian parameter. In
Fig.~\ref{secondderivativeenergy} the second derivative of the energy density is plotted in dependence of $\phi$ and shows a divergence for the
value $\phi=\phi_c\equiv\pi/4$ independent of $n$.  The singularity is ultimately due to the vanishing of the energy gap between the ground state and the
first excited state at the critical value $\phi_c$ with the modes $k=\frac{j\pi}{n+2}$, where $j$ runs from $0$ to $n+1$ .

\section{The spin correlations functions}
\label{Spincorrelation}

To obtain a generic spin correlation function we can adapt the strategy that we used to compute the energy density. Then applying Wick's
theorem~\cite{W1950} simplifies the issue further since it makes it possible to express any multi-body fermionic correlation
function in terms of two-body correlation functions. More precisely, it is possible to prove~\cite{BM1971} that defining for each site $j$,
two fermionic operators, $A_j$ and $B_j$, via
\begin{equation}
 \label{A&B}
 A_j=c_j+c_j^\dagger \qquad\textrm{and}\quad  B_j=c_j-c_j^\dagger\;,
\end{equation}
any spin correlation function can be written as an ordered
product of these operators. Hence, due to Wick's theorem, any spin correlation function can be written as a
combination of one- and two-body expectation values involving only operators $A_j$ and $B_k$ on the same or different sites.
With Eq.~(\ref{alphakbetak}) we obtain
\begin{eqnarray}
\label{correlations}
 \langle A_i \rangle & = &  0\;, \nonumber \\
 \langle B_i \rangle & = &  0\;, \nonumber \\
 \langle A_i A_k\rangle  & = & \delta_{ik}\;, \nonumber \\
 \langle B_i B_k\rangle  & = & -\delta_{ik}\;,  \\
 \langle B_i A_k\rangle  & = & G_{i,k}(n,\phi)\;. \nonumber
\end{eqnarray}
The fact that we have that both $\langle A_i \rangle = \langle B_i \rangle=0$ and  $\langle A_i A_k\rangle=\langle B_i B_k\rangle =0$
for $i \neq k$ has several important consequences.
In fact, let us consider a spin correlation function associated with an operator that is the product of many local spin operators, each one acting
onto different spins, in which $\sigma_j^x$ and/or $\sigma_j^y$  appears an odd number of times on different sites. To this operator we may
associate a fermionic operator made by a different number of $A_j$ and $B_j$ operators acting onto different spins. Therefore, when we apply the
Wick's theorem,
we have an expectation value of a single fermionic operator and/or an expectation value of two operators of the same kind onto different
spins. Hence, taking into account Eq.~(\ref{correlations}), such spin correlation functions have to vanish.
Consequently, the only correlation function that can be different
from zero are the ones associated with an operator that is a product of local spin operators in which both $\sigma_j^x$ and $\sigma_j^y$ appear an
even number of times.

To obtain the explicit expression of the non-zero spin correlation functions we need to evaluate $G_{i,k}(n,\phi)$. At first we note
that, in the thermodynamic limit, the $G_{i,k}(n,\phi)$ must be independent from the choice of $i$ and $k$ but may depend on
their relative distance \mbox{$r=i-k$}. With eq.~(\ref{alphakbetak}) we find $G_{i,k}(n,\phi)=G_{r}(n,\phi)$ with
\begin{equation}
 \!\!G_r(n,\phi)\!=\!\frac{1}{\pi}\! \int_0^\pi\!\!
\frac{\cos(\!k(\!n\!+\!1\!+\!r\!)\!)\!\cos\phi\!-\!\cos(\!k(\!r\!-\!1\!)\!) \sin\phi}{\sqrt{1-\cos((n+2)k)\! \sin(2\phi)}} dk \; .
\end{equation}
Solving this integral we find that if $r\neq l(n+2)+1$, where $l$ is an integer number that runs from $-\infty$ to $\infty$,
then the $G_{r}(n,\phi)$ vanishes for all values of $\phi$. This fact, as we show in Sec.~\ref{Entanglementproperties}, plays a fundamental
role in the behavior of the entanglement property among different spins.

Obviously, from Eq.~(\ref{correlations}) and the explicit expressions $G_{i,k}(n,\phi)$ one can recover all spin correlation functions of interest.
Here we wish to point out some interesting results about some specific ones.

If one allows for a magnetization along the $z$ direction, i.e. $\langle \sigma_j^z \rangle$, one finds that it equals $G_{0}(n,\phi)$ and,
therefore, vanishes identically for all possible values of $\phi$ and $n$. Let us consider two-body spin correlation functions that can be written
as $\langle \sigma_i^\mu \sigma_{i+r}^\mu\rangle$ with $\mu=x,y,z$.
If  $\mu$ coincide with $z$ the correlation function can be written as
\begin{equation}
 \langle \sigma_i^z \sigma_{i+r}^z\rangle= G_{0}(n,\phi)-G_{r}(n,\phi)G_{-r}(n,\phi) \;.
\end{equation}
Since $G_{r}(n,\phi)$ with $r \neq l(2+n)+1$ vanishes we find that
\begin{equation}
 \label{zcorr}
 \langle \sigma_i^z \sigma_{i+r}^z\rangle=0
\end{equation}
for all values of $n$ and $\phi$. Setting $\mu=x,y$ the spin correlation functions are given by the determinant
\begin{equation}
 \label{correlationmatrixx}
\!\! \!\!\!\!\langle \sigma_i^x \sigma_{i+r}^x\rangle\!=\!
 \left|
 \begin{array}{cccc}
 \! G_{-1}(n,\phi) & G_{-2}(n,\phi) &\! \cdots \!& \!\!G_{-r}(n,\phi)\! \\
 \! G_{-2}(n,\phi) & G_{-1}(n,\phi) & \!\cdots \!& G_{-r+1}(n,\phi)\!\! \\
 \! \vdots & \vdots & \!\ddots \!& \vdots\! \\
 \! G_{-r}(n,\phi) &\!\! G_{-r+1}(n,\phi) \!\!& \!\cdots\! &\!\! G_{-1}(n,\phi)\!
 \end{array}
\right|\;,
\end{equation}
\begin{equation}
 \label{correlationmatriyy}
\!\! \!\!\!\!\langle \sigma_i^y \sigma_{i+r}^y\rangle\!=\!
 \left|
 \begin{array}{cccc}
 \! G_{1}(n,\phi) & G_{2}(n,\phi) &\! \cdots \!& \!\!G_{r}(n,\phi)\! \\
 \! G_{2}(n,\phi) & G_{1}(n,\phi) & \!\cdots \!& \!\!G_{r-1}(n,\phi)\! \\
 \! \vdots & \vdots & \!\ddots \!& \vdots\! \\
 \! G_{r}(n,\phi) & G_{r-1}(n,\phi) & \!\cdots\! & \!\!G_{1}(n,\phi)\!
 \end{array}
\right|\;.
\end{equation}
Numerical evaluations  reveal that $\langle \sigma_i^x \sigma_{i+r}^x\rangle$
is non-vanishing only when $r$ is an integer multiple of $n+2$,
in strong contrast to the correlation function  $\langle \sigma_i^y \sigma_{i+r}^y\rangle$, which is always non-zero. It changes from negative to
positive values in the case $r$ varies from odd to even values. This is expected due to the anti-ferromagnetic nature of the Ising interaction.

\section{The order parameters}
\label{Orderparameters}

As we have seen in Sec.~\ref{Solution}, the behavior of the second derivative of the ground state energy density shows a phase
transition at $\phi=\phi_c\equiv \pi/4$ for all $n$. Now we characterize the properties of these two phases via the help of the spin correlation
functions (Sec.~\ref{Spincorrelation}).

Let us start from the phase $\phi>\phi_c$, i.e. when the system is dominated by a two-body anti-ferromagnetic Ising interaction along the $y$ spin
direction.  Due to the $Z_2$ symmetry of the Hamiltonian~(\ref{Hamiltonian}) we cannot compute the staggered magnetization by directly applying the
definition
\mbox{ $ m_y= (-1)^j \langle \sigma_j^y \rangle$} since this gives always a vanishing result. Approaching the problem we may first evaluate the
value of the magnetization with respect to its relation to the long distance correlation function along the same spin direction, i.e.
\begin{equation}
 \label{staggeredmagnetization}
 m_y=\sqrt{\lim_{r\rightarrow \infty} (-1)^r \langle \sigma_i^y \sigma_{i+r}^y\rangle}\;.
\end{equation}
This can be evaluated via the help of Eq.~(\ref{correlationmatriyy}). We have computed for different $n$ numerically the quantity
$(-1)^r \langle \sigma_i^y \sigma_{i+r}^y\rangle$ with $r$ up to 200, showing that an increase of the distance $r$ results only in a very small
variation of $m_y$ (of a factor less than $10^{-8}$) for each value of $\phi>\frac{\pi}{4}$.

\begin{figure}[t]
\includegraphics[width=0.49\textwidth]{newfig2.eps}
\caption{(Color online) Behavior of magnetic order parameter in the Ising phase $\phi>\phi_c$ plotted for $n=1,2,\dots,6$: red (uppermost curve)
$n=1$; blue $n=2$;
green $n=3$; black $n=4$; magenta $n=5$; orange (lowest curve) $n=6$ . The dots represent the numerical
results of $m_y$ for $r$ going to infinity,  Eq.~(\ref{staggeredmagnetization}), whereas the curves corresponds to the guessed function of the
staggered magnetization $m_y^{(n)}$, Eq.(\ref{staggeredmagnetizationformula}).}
\label{staggeredmagnetizationfig}
\end{figure}

The results that we have obtained for different $n$ and $\phi$ are plotted in Fig.~(\ref{staggeredmagnetizationfig}). This shows the presence of an
anti-ferromagnetic phase along the $y$-direction for $\phi>\phi_c$ independent of the value of $n$. However, differently from what happens for the
second derivative of the density of the ground state energy, the staggered magnetization shows a clear dependence on $n$. Analyzing the numerical
data we can conclude that the staggered magnetization has the following dependence on $\phi\ge \phi_c$ and $n$:
\begin{equation}
 \label{staggeredmagnetizationformula}
 m_y^{(n)}=\left(1-\tan(\phi)^{-2}\right)^{\frac{n+2}{8}} \; .
\end{equation}
From that we can deduce the critical exponent $\beta$ over $n$
\begin{equation}
 \label{beta}
 \beta(n)=\frac{n+2}{8}\;.
\end{equation}
The fact that the critical exponent $\beta$ depends on $n$ means that the class of symmetry to which the models given by the
Hamiltonian~(\ref{Hamiltonian}) belongs depends on $n$.

The situation changes drastically when we move in the phase below the quantum critical point $\phi<\phi_c$. In this phase our Hamiltonian is
dominated by the many-body interaction terms and $m_y$ drops to zero for any $n$. It is not straightforward to find a proper candidate or the
role of order parameter as it was for the anti-ferromagnetic phase discussed above. However, after an heavy numerical analysis we were able to
obtain a clear picture on the ongoing physics of the system.

For a system with odd $n$ we can define a string order parameter as
\begin{eqnarray}
\label{stringorderparameter}
 S_n&=&\sqrt{\lim_{r \rightarrow \infty} \langle \sigma_1^x \sigma_2^y \sigma_3^x\! \cdots\! \sigma_{n+1}^y \mathcal{O}  \sigma_{r-n+1}^y\! \cdots\!
 \sigma_{r-2}^x \sigma_{r-1}^y \sigma_{r}^x\rangle}\;,\nonumber\\
\end{eqnarray}
where the operator $\mathcal{O}=O^z_{n+1,r-2(n+1)}$. In Fig.~\ref{stringorderparameterfig} the behavior of this string order parameter $S_n$ for
$n=1,3,5$ is plotted. The existence of such a non-vanishing string order parameter can be traced back to the presence of diverging localizable
entanglement~\cite{PVMC2005,CR2005}. This signals the presence of a symmetry protected topological order.

\begin{figure}[t]
\includegraphics[width=0.49\textwidth]{newfig3.eps}
\caption{(Color online) Behavior of the string order parameter for $\phi<\phi_c$ for $n=1,3,5$: black (upper curve) $n=1$;  red (middle curve) $n=3$;
blue (lower curve) $n=5$. The dots represent the numerical
results of the string order parameter $S_n$ given in Eq.~(\ref{stringorderparameter}), whereas the curves correspond to the behavior of the string
order parameter $S^{(n)}$ defined in Eq.~(\ref{BneOn}).}
\label{stringorderparameterfig}
\end{figure}

For even $n$ we find that the phase is a nematic one thus we can define the following order parameter (since the system is translation invariant
the quantity is understood to not depend on the particular $i$)
\begin{equation}
\label{blockorderparameter}
\mathcal{B}_{n}=\langle \mathcal{O}_{i,n}\rangle=\langle \sigma_i^x \sigma_{i+1}^y \sigma_{i+2}^x\! \cdots\! \sigma_{i+n}^x  \rangle
\end{equation}
As in the staggered magnetic order phase $\mathcal{B}_n$ cannot be evaluated directly since it vanishes (for any even $n$ the operators
$\sigma_i^x$ or $\sigma_i^y$ appear an odd number of times). Again we can circumvent this problem by defining
\begin{equation}
\label{blockorderparameter2}
B_n=\sqrt{\lim_{r \rightarrow \infty }\langle \mathcal{O}_{i,n} \mathcal{O}_{i+r,n} \rangle}\;.
\end{equation}
In Fig.~\ref{blockmagnetizationfig} we plotted the behavior of $B_n$ for $n=2,4,6$.

\begin{figure}[t]
\includegraphics[width=0.49\textwidth]{newfig4.eps}
\caption{(Colour online) Behavior of the nematic order parameter for \mbox{$\phi<\phi_c$} for $n=2,4,6$; black (upper curve) $n=2$;  red (middle curve) $n=4$;
blue (lower curve) $n=6$. The dots represent the
numerical results of the nematic order parameter $B_n$, Eq.~(\ref{blockorderparameter2}), whereas the curves correspond to nematic order
parameter $B^{(n)}$, Eq.~(\ref{BneOn}).}
\label{blockmagnetizationfig}
\end{figure}

Analyzing the numerical data obtained for both defined string order parameters, $S_n$ and $B_n$, we find finally the same dependence on $n$
and $\phi$, i.e.
\begin{eqnarray}\label{BneOn}
 S^{(n)}&=&\left(1-\tan(\phi)^{2}\right)^{\frac{n+2}{8}}  \nonumber \\
 B^{(n)}&=&\left(1-\tan(\phi)^{2}\right)^{\frac{n+2}{8}} \; .
\end{eqnarray}

Summarizing all results we can formulate a general concise formula for all order parameters of the whole class of models given by the
Hamiltonian~(\ref{Hamiltonian}):
\begin{eqnarray}\label{generalOrderPar}
\textrm{Order Parameter}&=& \left(1-\tan(\phi)^{-2 sgn(\phi-\frac{\pi}{4})}\right)^{\frac{n+2}{8}}\;.\nonumber\\
\end{eqnarray}
Moreover, the existence of a duality, i.e. a transformation that brings the order parameters before and after the critical point in relation, is
thus proven.

In summary, we find that for both phases we can define order parameters that each is ruled by the dominated interactions, i.e. Ising interaction or
multi-body cluster interaction. In the multi-body cluster phase a strong dependence on the size of the cluster $n+2$ is present revealing either a
nematic phase (even $n$) or a topologically ordered phase (odd $n$).

\section{The entanglement properties}
\label{Entanglementproperties}

In this section we analyze the entanglement properties between adjacent spins as well as between a block of spins and the remaining part of the
chain. Despite the complexity of the class of models under investigation we obtain general results showing the relevance of the entanglement
features in these complex matter systems.

The object of matter is the reduced density of $m$ spins, which is obtained by taking the trace over all remaining spins of the ground state.
Any such reduced density matrix we can decompose by the spin correlation functions
\begin{equation}
 \label{densitymatrix}
 \rho_m^{(n)}=\frac{1}{2^m} \sum_{\alpha_1,\dots,\alpha_m} \langle \sigma_1^{\alpha_1}\sigma_2^{\alpha_2}\cdots\sigma_m^{\alpha_m}\rangle
 \sigma_1^{\alpha_1}\sigma_2^{\alpha_2}\cdots\sigma_k^{\alpha_k}\; ,
\end{equation}
where $\alpha_i$ runs from $0,x,y,z$ and $\sigma_i^{0}$ denotes the identity.

The next subsection introduces the concept of different types of multipartite entanglement. Then we compute the entanglement properties of
adjacent spins and the entanglement between a block of spins and the remaining part of the chain.

\subsection{Definition of hierarchies of multipartite separability}

The quantum separability problem reduces for bipartite entangled systems to the question of whether the state is entangled or not. In the
multi-partite case the problem is more involved. First, there exist different hierarchies of separability since an $n$-partite entangled
state $\rho$ may be a convex combination of pure entangled states with maximally $k$ entangled particles. Any tripartite pure state, e.g., can be
written as
\begin{eqnarray}
|\psi_{k=3}\rangle&=&|\phi_A\rangle\otimes|\phi_B\rangle\otimes|\phi_C\rangle\nonumber\\
|\psi_{k=2}\rangle&=&|\phi_A\rangle\otimes|\phi_{BC}\rangle,\quad|\phi_B\rangle\otimes|\phi_{AC}\rangle\nonumber\\
&&\textrm{or}\quad |\phi_{AB}\rangle\otimes|\phi_{C}\rangle\nonumber\\
|\psi_{k=1}\rangle &=&|\psi\rangle_{ABC}
\end{eqnarray}
where $k$ gives the number of partitions dubbed the $k$-separability. In general a pure state $\ket{\Psi^k}$ is called $k$-separable, if and only if
it can be written as a tensor product of $k$ factors $\ket{\psi_i}$, each of which describes one or several subsystems, i.e.
\begin{eqnarray}\label{k-separability}
\ket{\Psi^k}&=&|\psi_1\rangle\otimes\ket{\psi_2}\otimes\dots\otimes\ket{\psi_k}\;=\;|\psi_1\psi_2\dots\psi_k\rangle \; .\end{eqnarray}
A mixed state $\rho$ is called $k$-separable, if and only if it can be decomposed into a mixture of $k$-separable pure states
\begin{eqnarray} \rho = \sum_i p_i \ket{\Psi_i^k}\bra{\Psi_i^k}
\end{eqnarray}
where all $\ket{\Psi_i^k}$ are $k$-separable (possibly with respect to different $k$-partitions) and the $p_i$ form a probability distribution.
An $n$-partite state (pure or mixed) is called fully separable if and only if it is $n$-separable. It is called \textit{genuinely multi-partite
entangled} if and only if it is not bi-separable (2-separable). If neither of these is the case, the state is called \textit{partially}
multipartite entangled or \textit{partially} multipartite separable. Note that obviously a $k=3$-separable state is necessarily also
$k=2$-separable, thus $k$-separable states have a nested-convex structure.

In particular, note that the following tripartite mixed state
\begin{eqnarray}
\rho&=&\;\sum_i p_i\; |\psi_i\rangle_{AB}\langle\psi_i|_{AB}\otimes|\sigma_i\rangle_C\langle \sigma_i|_C\nonumber\\&& +\sum_i q_i\;
|\chi_i\rangle_{AC}\langle\chi_i|_{AC}\otimes|\tau_i\rangle_B\langle \tau_i|_B\nonumber\\
&&+\sum_i r_i\; |\xi_i\rangle_{BC}\langle\xi_i|_{BC}\otimes|\omega_i\rangle_A\langle \omega_i|_A
\end{eqnarray}
with $p_i,q_i,r_i\geq 0$ and $\sum p_i+q_i+r_i=1$ is bi-separable though it is not bi-separable with respect to a certain splitting. This property
and the fact that the convex sum of pure states is not unique are the reasons why it is hard to detect genuine multipartite entanglement, i.e. a
state that cannot be written in the above form. Consequently, the entanglement characterization of multi-partite states needs more than the
combination of bipartite entanglement criteria~\cite{HMGHframework}.

\subsection{Entanglement properties among adjacent spins}

Let us start by analyzing the case of $m$ adjacent spins thus having a maximum distance of $r=m-1$. Then all spin correlation functions can be
expressed by $G_{r}(n,\phi)$ with $-(m-1)<r<m-1$.

\begin{theorem}
If the number of adjacent spins $m$ is smaller than the cluster size, i.e. $m<n+2$, then all $k\leq m$-partite entanglement vanishes, i.e. the
reduced state is $k\leq m$-separable. If the number of adjacent spins equals the cluster size, i.e. $k=n+2$, then there exists a finite range of
values of $\phi$ for which the reduced density matrix to this set of
spins is genuinely $n+2$-partite entangled (plotted in Fig.~\ref{multipartiteentanglementfig}).
\end{theorem}

\textbf{Proof:} Let us start with $m<n+2$. In Sec.~\ref{Spincorrelation} we have computed all spin correlation functions $G_r(n,\phi)$ and found
that they vanish if $r\not=(n+2)l+1$. The reduced density matrix $\rho_m^{(n)}$ depends only on a single function, i.e. $G_1(n,\phi)$. This implies
that only spin correlation functions that are different from
zero are the ones along the $y$-direction. Consequently, the reduced matrix $\rho_m^{(n)}$ is a mixture of states being eigenvectors to the
single-spin operators $\sigma_j^y$. Applying the following local unitary operators
\begin{equation}
 \label{Unitary}
 U_j=\exp\left(-i \frac{\pi}{4} \sigma_j^x\right) \; ,
\end{equation}
brings the density matrix $\rho_m^{(n)}$ of $m$ adjacent spins into a diagonal form which obviously is separable.

\begin{figure}[t]
\includegraphics[width=0.49\textwidth]{newfig5.eps}
\caption{(Color online) Dependence of the genuine multipartite concurrence $C_{gm}^{(n+2)}$ as function of the weighted interactions $\phi$ for
different $n$ that runs from $1$ (highest curve) to $12$ (lowest curve). Note that only for $n=1$ genuine tripartite entanglement is non-zero
before and after the critical point and, generally, genuine $n+2$-partite entanglement decrease with increasing cluster size.}
\label{multipartiteentanglementfig}
\end{figure}

In the case where the adjacent spins equals the cluster size, $m=n+2$, the reduced density matrix $\rho_{n+2}^{(n)}$ depends on $G_1(n,\phi)$ and
$G_{-(n+1)}(n,\phi)$ that corresponds to the spin cluster correlation function $\langle \sigma_k^x O_{k,n}^z\sigma_{k+n+1}^x \rangle$. Again
applying the above defined local unitary operators $U_j$ to each spin we obtain a reduced density matrix $\rho_m^{(n)}$ that has an
X-form~\cite{YE2007}, i.e. only entries on both diagonals are nonzero. It has been shown that if a density matrix can be written in such an
$X$-form, the genuine multipartite entanglement can be exactly evaluated by a certain measure, dubbed genuine multipartite concurrence introduced
in Refs.~\cite{HH2008,MCCSGH2011,HHBE2012}. Thus, by applying the above defined local unitaries we find the following expression for the genuine
$(n+2)$-partite concurrence for any $n$ and $\phi$
\begin{eqnarray}\label{genuinemltipartiteconcurrence}
\lefteqn{C_{gm}^{(n+2)}(\phi)\;=}\nonumber\\
&&\max[0,\frac{1}{2^{n+1}} \left(1-G_{1}(n,\phi)\right)^{n+1}\cdot \left(G_{-(n+1)}(n,\phi) +1\right)\nonumber\\
&&\qquad\qquad\qquad -1 ]\;.
\end{eqnarray}

In Fig.~\ref{multipartiteentanglementfig} we have plotted the genuine $(n+2)$-partite concurrence for $n=1,\dots,12$ and find for certain $\phi$
non-zero values. Q.E.D.\\
\\
Looking more carefully at the curves, one observes a similar behavior for all $n$ and, except for $n=1$, a non-zero value of genuine
$(n+2)$-partite multipartite is only obtained in the Ising phase. Moreover, the genuine $(n+2)$-partite concurrence is always smaller for bigger
cluster sizes. That proves that the entanglement in the ground state becomes robust against the Ising-interaction (remember the ground state of
$\phi=0$ is a graph state and for $\phi=\frac{\pi}{2}$ a totally factorized state~\cite{GAI2008,GAI2009,GAI2010}). Consequently, higher cluster
sizes allow for better properties for running quantum algorithms.

\begin{figure}[t]
\includegraphics[width=0.49\textwidth]{newfig6.eps}
\caption{(Color online) Behavior of $\frac{\pi}{2}-\phi_\textrm{max}^{(n)}$ as function of $n$ where the maximization is taken for the genuine
multipartite concurrence. The red dots are the result of the numerical maximization
for any $n$ while the black line represent the fit, obtained for large $n$, in  Eq.~(\ref{powerlawmax}).}
\label{multipartiteentanglementpositionfig}
\end{figure}

\begin{figure}[t]
\includegraphics[width=0.49\textwidth]{newfig7.eps}
\caption{(Color online) Dependence of the maximum value of the genuine multipartite concurrence $C_{gm}^{(n+2)}(\phi_\textrm{max}^{(n)})$ on the
cluster size $n+2$. The (red) dots are the results of the numerical maximization for any $n$ whereas the (black) line represent the fit obtained
for large $n$ presented in Eq.~(\ref{powerlawmax}).}
\label{multipartiteentanglementvaluefig}
\end{figure}

\begin{figure}[t]
\includegraphics[width=0.49\textwidth]{newfig8.eps}
\caption{(Color online) Dependence of $\frac{\pi}{2}-\phi_*^{(n)}$ as function of $n$. The (red) dots are the result of the numerical result
for specific cluster sizes $n+2$ whereas the (black) line represents the fit result obtained for large $n$ presented in Eq.~(\ref{powerlawmax1}).}
\label{multipartiteentanglementzerofig}
\end{figure}
In Fig.~\ref{multipartiteentanglementpositionfig} and Fig.~\ref{multipartiteentanglementvaluefig} a deeper analysis of the entanglement properties
of the reduced matrix can be found concerning the maximal value of the weight $\phi_\textrm{max}^{(n)}$ of the two interactions which corresponds to
the maximal reachable value of genuine $n+2$-partite concurrence $C_{gm}^{(n+2)}$. Both values show a similar dependence that for $n>10$ is in good
approximation given by
\begin{eqnarray}
 \label{powerlawmax}
\phi_\textrm{max}^{(n)}&=& \frac{\pi}{2}-\frac{3.1}{n} \nonumber \\
 C_{gm}^{(n+2)}(\phi_\textrm{max}^{(n)})&=&\frac{0.47}{n} \; ,
\end{eqnarray}
where the numerical coefficients are obtained by a best fit algorithm. Analogously, the point in which the genuine $(n+2)$-partite
entanglement becomes different from zero depends on the inverse of $n$, plotted in Fig.~(\ref{multipartiteentanglementzerofig}),
\begin{equation}
 \label{powerlawmax1}
 \phi_*^{(n)}= \frac{\pi}{2}-\frac{6.2}{n} \;.
\end{equation}
From these equations we immediately reveal an interesting relation between $\phi_\textrm{max}^{(n)}$ and $ \phi_*^{(n)}$, i.e.
\begin{equation}
 \label{powerlawmaxrelation}
 \left( \phi_*^{(n)}- \frac{\pi}{2}\right)=2 \left(\phi_\textrm{max}^{(n)}- \frac{\pi}{2}\right) \;,
\end{equation}
valid for large $n$.

In summary, these cluster-Ising models with different cluster sizes have interesting local entanglement properties. There is no bipartite,
tripartite,..., $n+1$ entanglement, but only for large enough values of Ising interaction $\phi>\frac{\pi}{4}$ one finds local entanglement,
in particular only genuine $n+2$-partite multipartite entanglement. In Ref.~\cite{HKN2006} the authors computed that the maximal value of maximal
possible entanglement of two adjacent spins in a translation invariant chain was found to give a (bipartite) concurrence of $C=0.434467$. This
optimal value serves for interpreting entanglement
values obtained for real physical systems. In the very same manner the maximal values of the multipartite entanglement quantified by the above
introduced genuine multipartite entanglement measure serves as an reference for real physical system exhibiting cluster and Ising interactions.

\subsection{Entanglement properties between a block of spins and the rest of the chain}

Another important property to analyze in multipartite systems concerns the entanglement features of a block of $m$ spins with the rest of the chain
and how it classifies to the holomorphic and anti-holomorphic sectors in conformal field theories.

For that purpose we have to compute the von Neumann entropy of the reduced density matrix of $m$ spins,
\begin{equation}
\label{VNEdefinition}
 S_{m}^{(n)}=Tr(\rho_m^{(n)} \log_2(\rho_m^{(n)}))\;.
\end{equation}
Using the methods developed in Ref.~\cite{VLRK2003,LRV2004} we find
\begin{equation}
 \label{VNEdefinition1}
 S_{m}^{(n)} = \sum_{j=1}^m H_{\textrm{Shannon}}\left(\frac{1+\nu_j}{2}\right)
\end{equation}
where $H_{\textrm{Shannon}}(x)$ is the Shannon entropy
\begin{equation}
 \label{Shannonentropy}
 H_{\textrm{Shannon}}(x)= -x \log_2(x) -(1-x) \log_2(1-x)\; ,
\end{equation}
and $\nu_j$ is the imaginary part of the eigenvalues of the matrix
\begin{equation}
\label{gammaprime}
 \Gamma'= \delta_{ij}-i \Gamma_m
\end{equation}
with
\begin{equation}
\label{gamma}
 \Gamma_m=\left( \begin{array}{cccc}
 \! \Pi_0 & \Pi_{-1} &\! \cdots \!&  \Pi_{-m+1} \! \\
 \! \Pi_{1} & \Pi_0 & \!\cdots \!&  \Pi_{-m+2}\! \\
 \! \vdots & \vdots & \!\ddots \!& \vdots\! \\
 \! \Pi_{m-1} &\Pi_{m-2} & \!\cdots\! & \Pi_0\!
 \end{array}
\right)
\end{equation}
and
\begin{equation}
\label{pi}
 \Pi_r=\left(
 \begin{array}{cc}
 0 & G_{r}(n,\phi) \\
 -G_{-r}(n,\phi) & 0 \\
 \end{array}
\right)\;.
\end{equation}

We have evaluated numerically the von Neumann entropy for blocks of length ranging from 2 to 200 spins at the critical point $\phi_c$ for
$n$ that runs from $1$ to $10$. The obtained values of the von Neumann entropy are displayed in Fig.~\ref{voneumannfig}.
\begin{figure}[t]
\includegraphics[width=0.49\textwidth]{newfig9.eps}
\caption{(Color online) Here the von Neumann entropy $S^{(n)}_m$, Eq.~(\ref{VNEdefinition}), in dependence of a block size $m$ for different
cluster sizes $n$ is plotted from which we fit the numerical solution of the von Neuman entropy, see Eq.~(\ref{numericalfitvonneumann}). The value
of $n$ runs from $1$ lowest (black) curve to $8$ the highest (pink) curve.}
\label{voneumannfig}
\end{figure}

Analyzing the numerical data we deduce
\begin{equation}
\label{numericalfitvonneumann}
 S_{m}^{(n)}\simeq(0.32+0.18\;n)\; \log_2 m+const(n)
\end{equation}
The multiplicative constant in front of the logarithmic term is known to be related to the central charge of the $1+1$ dimensional conformal
theory describing the critical behavior of
the chain via the relation~\cite{HLW1994}
\begin{equation}
 \label{cft}
 S_m = \frac{\mathsf{c}+\overline{\mathsf{c}}}{6}\; \log_2 m\;,
\end{equation}
where $\mathsf{c}$ and $\overline{\mathsf{c}}$ are the central charges of the so-called holomorphic and anti-holomorphic sectors of the conformal
field theory. Due to the existence of a duality in the system under investigation we have that $\mathsf{c}=\overline{\mathsf{c}}$ and hence, via
Eq.~(\ref{numericalfitvonneumann}) we
obtain
\begin{equation}
\label{centralcharge}
  \mathsf{c}\simeq 3\cdot (0.32+0.18\;n)\;.
\end{equation}
For two quantum one-dimensional systems to belong to the same universality class they need to have the same central charge. Since in our case we
find a dependence on $n$, this central charge, in addition to the critical exponent $\beta$, Eq.~(\ref{beta}), of the order parameters,
Eq.~(\ref{generalOrderPar}),
proves that the many-body cluster-Ising models fall into different classes with respect to their symmetries.

\section{Conclusions}
\label{Conclusions}

In summary, we have analytically solved, characterized and analyzed the properties of a family of models that we named $n$-cluster-Ising models.
These are models characterized by different cluster sizes ($n+2$) and different weighted cluster interaction and Ising interaction. We proved that
there occurs a phase transition exactly when both interactions are equally weighted and, interestingly, independent of the cluster size.

With respect to their symmetries the family of models falls into different classes proved via the dependence on $n$ of the critical exponent
$\beta$ of properly defined order parameters and the central charge of the holomorphic and anti-holomorphic sectors in conformal field theories.
In particular we find that the cluster phase has very different orderings for odd or even cluster size, namely a topological or a nematic order.
Since nematic order usually shows up only for non-analytically solvable systems these cluster-Ising models may become a prototype testing model for
exploiting the physical potential of nematic ordering of spins.

In the next step we have investigated how the apparent complexity of the ordering translates to the multipartite entanglement properties shared
among spins or block of spins with the rest of the system. Surprisingly, exactly all reduced density matrices with $m$ adjacent spins smaller than
the cluster size ($=\;n+2$ adjacent spins) posses no entanglement, whereas the reduced density matrices for exactly the cluster size ($n+2$)
possesses \textit{genuine} $n+2$-multipartite entanglement if the Ising interaction is strong enough, but not maximal
(see Fig.~\ref{multipartiteentanglementfig}). This absence of bipartite or $n-1$-partite multipartite entanglement is very different from other one
dimensional spin models, i.e. as the Ising one~\cite{OAFF2002,ON2002} or the $XY$-model~\cite{GH2013}. That computation was possible,
because the symmetries of the Hamiltonian constrain the state space in the Hilbert-space in a non-trivial way enabling even the computation of a
measure of genuine multipartite entanglement. From the quantum information perspective these results show that increasing the cluster size reduces
local entanglement and, herewith, the robustness of the performance of any quantum algorithm. From the perspective of comparison of different
condensed matter systems the family of models serves as a reference system of the possible amount of local genuine multipartite entanglement that
can be shared.

Our family of models can be generalized with respect to higher dimensions both in space and degrees of freedom (higher spins). These models may
become a good testing ground for non-trivial spin orderings and serve as a prototype for studying the potential of a quantum computer.

\section*{Acknowledgments} The authors
acknowledge gratefully the Austrian Science Fund (FWF-P23627-N16). We thank Benjamin Rogers for carefully reading the manuscript.

redpajama_set_name: RedPajamaArXiv


text:
The location: Isaak kills Louis (on a dock)
Q. What is it supposed to be on the show?
A. A dock, at Dexter's marina.
Q. Where is it supposed to be on the show?
A. Somewhere in Miami.
Q. When did we see it on the show?
A. In Episode 3, of Season 7, "Buck the System".
Ukrainian mob boss Isaak learns that his employee, Viktor (who murdered Mike Anderson), has been killed, and his body dumped at sea.
So he goes looking for the person who did it.
Tracking the GPS bracelet that Viktor was wearing, they zero in on a dock at Dexter's marina.
But when they reach Dexter's boat (the Slice of Life), instead of Dexter, they find Louis on the boat. Louis was planning to get petty revenge on Dexter by drilling holes in his boat and sinking it.
At first, Louis pretends to be the owner of the boat. But when Isaak threatens to drill his eyes out, Louis tells them it really belongs to Dexter Morgan, who works at Miami Metro Homicide.
Before leaving, Isaak turns and shoots Louis in the head. His blood spills onto the deck of Dexter's boat.
We see the dock again at the start of Episode 5 ("Swim Deep"), where Dexter is cleaning his boat and having an imaginary conversation with Harry about Debra.
Then Dexter discovers blood, and knows that someone has been on his boat.
It shows up later in Episode 8 ("Argentina"), when LaGuerta (still investigating the Bay Harbor Butcher case) shows up at night and looks at the name on the side of his boat: "The Slice of Life".
Q. What is it actually in real life?
A. A dock, adjacent to a marina.
Q. Where can I find it in real life?
A. This was shot near the southeast corner of the Alamitos Marina, in Long Beach, CA.
It's in a somewhat remote spot in the otherwise busy marina, at very end of Marina Drive, at the far tip of a marina jetty.
You'll find this dock right behind the blue City of Long Beach Marine Bureau building, at 205 Marina Drive (which is also home to the Long Beach Police Dept.'s Marine Patrol).
The Slice of Life was docked at the narrow, southwest tip of this dock.
If you want to visit the spot, be sure to check a map -- the jigsaw puzzle shape of the marina can get a little confusing without one. And finding this dock can get tricky, because there is more than one Marina Drive in this area. In fact, this Marina Drive actually crosses another one: N. Marina Drive, which itself later turns into E. Marina Drive.
All of these Marina Drives run along outside edge of the Alamitos Marina, marking its northern and eastern borders.
The jetty is tucked away behind the Alamitos Landing shopping/dining center.
It's about a half a mile southwest of another Dexter location this year: the Schooner or Later restaurant.
It's also close to Shopkeeper Road, where they filmed the "search for bodies" scene in the second episode, as well as the spot where they filmed a bus accident scene later in the season.
Also, don't confuse this Alamitos Marina with Long Beach's Shoreline Marina (another spot where Dexter films a lot).
The two marinas are five miles apart. Alamitos Marina is just west of Pacific Coast Highway, right across the San Gabriel River channel from Seal Beach.
(A bit of trivia: part of the opening credits for "Gilligan's Island" were shot at this same location.)
I shot the photos below in October 2012.
Here is an aerial photo of the location. Here is a Bing StreetSide View.
And here is a map link.
Q. How the heck did you figure out where it was?
A. In the early seasons, I usually had to hunt down the locations after viewing the episodes, using clues from the various scenes. By the now, though, I've developed a small group of fans, spies & tipsters who kept an eye out for Dexter filming in their neighborhoods, and would let me know in advance when something was about to film there.
Between those reports, my own personal reconnaissance around town, and a few new resources I discovered, by the time the first episode airs, I already know most (but not all) of the filming locations, and only need to watch the episodes and match up the scenes with the correct locations.
This group of helpful fans includes Rick, Ellen, Elaine, Mia, Joel, Susan, Eric, Jeff, Kerry & others. My thanks to all of them.
I had two clues to work with on this one. One was the view in the background, which I recognized as Naples Island. It wasn't that hard to match up the houses seen in the background with aerial photos of the island, and then just draw a sightline from the houses to the likely camera location. However, when I did that, it put me a little too far to the west.
But then, in the episode, they showed us an actual aerial photo of the dock on someone's cell phone:
The dock has a distinctive shape, and since I knew the approximate area, it was easy to then match up that particular dock with Google's aerial photos.
I then visited the dock to shoot the photos you see above, and confirmed the details that matched the scene.
By Episode - By Category - By Geographical Location - Clickable Map of All Dexter Locations - Go To Main Menu
The Dexter screenshots from the show and all related characters & elements are trademarks of and © Showtime.
All other photos & text are Copyright © 2020-Gary Wayne and may not be used without written permission.
Return to Seeing-Stars.com
Looking for something in particular? Search the Seeing-Stars website!


text:
Q: JShint Ant task I am currently using the jshint plug-in in Eclipse to check the code for compliance with coding standards.
This project is built using Ant and I am trying to find a jshint Ant task (https://github.com/philmander/ant-jshint is no longer being maintained so that it is out of the question) to include jshint checks as part of the build.
My question is, is there any library that provides jshint for Ant, and if not what plug-in for Eclipse could also provide an ant task for checking my Javascript style?

A: I only know of the jshint-eclipse plug-in (http://github.eclipsesource.com/jshint-eclipse/). It creates error and warning markers within the IDE as you save your Javascript files but does not provide an Ant task.
If you don't mind implementing an Ant task by yourself, you should be able to use its JSHint class to accomplish the task.

redpajama_set_name: RedPajamaStackExchange


could you be a little more spcific? you meen a meshing tool like the meta ball object? or meshing like booleans? what exactly do you mean better meshing tools? the only reason i as is because im looking for plugin ideas to create. let me know.


New tools to help with social media marketing are popping up everywhere. But many small businesses and nonprofits just don't have the time to keep up and research all the options. Don't you wish you had someone to tell you about the tools that are proven to be really easy and useful? We get it! That's why last week we asked our Facebook fans, "What tool(s) do you use to help with your social media marketing on Facebook, Twitter, etc.?" Now, the results are in.
HootSuite was by far the no. 1 tool mentioned by our Facebook fan participants. If you haven't heard of it, HootSuite is a free social media dashboard that you can use to manage and measure your social network activity. You can schedule Facebook messages and tweets, track brand mentions, and analyze your social media traffic. And for a more comprehensive, one-stop-view of your social media marketing results, you can easily add your email campaign results into your HootSuite dashboard with Constant Contact's HootSuite app.
Some of the other social media marketing tools mentioned by our Facebook fans included Constant Contact's NutshellMail and Simple Share tools, Ping.fm, and Mywebees.
Have you tried any of these? Is HootSuite your top tool? Share your top tool here or add it to the Facebook discussion.
As a member of Constant Contact's distance learning team, I develop and host webinars that help small nonprofits and businesses learn best practices for online marketing. I hold an MBA in small business management, owned a marketing service business, and have more than 10 years of experience helping nonprofits and small businesses succeed.
I have been using Tweetdeck, and knew about Hootsuite. After reading this and exploring the Hootsuite services, I think I'm going to install the free version of Hootsuite and give it a try.


If you've been arrested for a DUI (driving the influence) or DWI (driving while intoxicated) because of an alcohol or drug arrest, you should consider your options. You're going to lose your license, get large fines, and get jail time, right? Not always, because there are some cases where you can beat a DUI charge. Now, if this is after multiple violations, if someone was hurt while you were driving under the influence, or it's deemed you risked minors, you may get an aggravated DUI charge. Just like it sounds, it's a bigger penalty than the initial DUI charge. This means you face larger fines, longer suspensions, and extended jail time. There are ways to beat the charge. Do you need a lawyer immediately? It would be easy to say, "hire a lawyer immediately, you have to." But in most DUI arraignments, where you can decide to plead not guilty or guilty, you may be okay without a lawyer initially. You will sometimes not even have to post bail unless you do not want to spend any time at all in jail. On the other hand, aggravated DUI charges are very serious. Instead of a 1-2 year license suspension, you can double or triple that. Instead of $1,000, you can pay several thousand more. Instead of limited jail time, you might face an extended prison sentence. This depends on the nature of the arrest. Aggravated DUI charges are generally considered felonies, while regular DUI charges are usually misdemeanors. In some cases, you can handle a misdemeanor initially by yourself, hiring a lawyer to help you if you want to fight the charge. Why do you need a lawyer? If you want to beat an aggravated DUI charge--which is hard but far from impossible--you immediately need help from an experienced DUI lawyer. He or she can help you decide how to plead, what chances you have in fighting the charges, and negotiating with prosecutors for a lesser charge. What options do you have? For an aggravated DUI charge, you can plead guilty, plea bargain for a reduced charge, ask for a trial before a judge or demand a jury trial. These may sound simple, but take for example the judge or jury question. How do you know if this judge will be lenient, especially if he or she regularly hears DUI defenses? How will a jury look to you if your blood alcohol content was incredibly high and you hurt someone? It depends on the case. This is where hiring a professional saves you time, money, and penalties like jail time.


text:
J. Murray Bartels (born Julius Murray Bartels; July 15, 1871 – October 5, 1944) was a  New York City-based dealer and auctioneer of rare postage stamps. He was also well known for his knowledge of United States postal stationery.

Family
Barthels was born in Warrenton, Fauquier County, Virginia, one of six or so siblings born to Hermann Friedrich Bartels and Sally Innes Bartels. His father was born in Germany.

Collecting interests

Bartels was primarily interested in United States postal stationery and became an expert on the subject. He published the result of his studies in J.M. Bartels and Co.'s Catalogue and Reference List of the Stamped Envelopes, Wrappers and Letter Sheets in 1897, and several editions of Envelopes of the United States, from 1910-38.

In 1943, he published a two volume set on stamped envelopes and wrappers.<ref>P.H. Thorp, ed.; Bartels Catalogue of the Stamped Envelopes and Wrappers of the United States and Possessions", Fifth Edition, 1943.</ref> He published philatelic literature on other philatelic subjects, such as, The Postage Stamps of the Philippines (co-authored with F.A. Foster and F.L. Palmer, in 1904), Bartel's Checklist of Canal Zone Stamps, in 1906 and 1908, and United States Virgin Islands'' (co-authored with Bertram William Henry Poole) in 1917.

Philatelic activity
Bartels conducted 337 philatelic auctions. Among his most important sales were portions of the significant portions of the Clarence Eagle and Arthur Hind prize-winning collections.

Honors and awards
Bartels was named to the American Philatelic Society Hall of Fame in 1946.

Legacy
Prescott Holden Thorp continued Bartels work with his publishing of "Thorp-Bartels" catalog editions.

See also
 Philately
 Philatelic literature
 J. Murray Bartels profile, archive.org; accessed December 18, 2017.

References

1871 births
1944 deaths
Philatelic literature
American philatelists
American stamp dealers
People from Warrenton, Virginia
Businesspeople from New York City
American Philatelic Society
Place of death missing
American people of German descent

redpajama_set_name: RedPajamaWikipedia


If Triglav is The King of the Julian Alps then Skrlatica is certainly his Queen. Wife of the King must be beautiful and powerful but still elegant with strong appearance. And Skrlatica is just like that, it impresses anyone who puts its sight on it. She is enchanting just like her King. Together they rule above the most beautiful Slovenian Alpine valley; Vrata valley.
Skrlatica is second highest Slovenian peak and third highest in Julian Alps, behind Triglav (2864m) and Montaz (Iof di Montasio, 2754m). It is highest peak of Martuljek - Skrlatica group, which contains most of the wildest peaks in Julian Alps. Skrlatica, just like the whole group and Julian Alps in general, is very steep. Its sides fall deep into the valleys below with high faces and cliffs. On the northwest is Krnica valley, over 1600m lower. Above it Skrlatica shows it most powerful side, magnificent 700m NW face. Together with the faces of its southwestern neighbors; the nearby Rakova Spica (2545m) and Rogljica (2547m) it forms one of the most beautiful walls in Slovene mountains. Beside these two ridge peaks first real neighbor of Skrlatica in this direction is monumental Dolkova Spica (2591m). Between it, Rakova Spica, Rogljica and Skrlatica is large Zadnji Dolek (Last Basin) whose sides, below the cliffs of surrounding peaks, and bottom is strewn with scree and large boulders. On the southeast is Vrata valley, over 1700m lower. Towards it Skrlatica falls with around 600m high torn cliffs. From anywhere you look Skrlatica is fortress mountain and it reminds of Dolomite mountains. Closest neighbor on the northeast is wild Visoki Rokav (2646m) (High Rokav). Between them is wild and airy teethed ridge. Over it Skrlatica is connected to Martuljek group. On the east is Spodnji Rokav (2500m) (Lower Rokav). With these two Rokav's Skrlatica closes wild V Kotlu (In the Cauldron) basin that is surrounded with these wild peaks and filled with scree. This is one of the wildest corners of Julian Alps.
Skrlatica group is placed between Martuljek group, on the north, with which is forms larger group, and Prisojnik (2547m) - Razor (2601m) group, on the south.
Beside Skrlatica only Dolkova Spica and Spik have been reached by marked (secured) paths. This group has least number of paths. All other peaks are reserved for climbers and alpinists, what makes this group their true preserved playground and most untouched area of Julian Alps.
On the first look Skrlatica does not have a week point but anyway a secured trail found its way to the summit, via southern ridge, which is above Vrata valley. If there wasn't a trail to the summit, Skrlatica would be one of the, if not THE toughest Slovenian mountain. It resisted conquering for a long time. Many famous alpinists of 19th century tried and failed. Finally in 1880, famous explorer of Julian Alps, Dr. Julius Kugy and two guides from Trenta valley, Andrej Komac and Matija Kravanja, climbed it. Today's path follows their footsteps. Even today Skrlatica is described as tough mountain, reserved for experienced mountaineers.
There are 3 different routes to climb Skrlatica, each ascending from a different valley. Vrata valley route is classic, used by most mountaineers. It is also shortest and easiest of 3. Krnica valley route is harder and includes two tough ferratta sections (secured paths with pegs and fixed steel ropes). First is Kriska Stena face and the other is summit climb. Trenta valley route is longest but less technical than Krnica valley route. They join on top of Kriska Stena face. Summit climb is the same for all routes as Krnica and Trenta valley routes meet Vrata valley route in Zadnji Dolek basin at the southern foot of Skrlatica.
View from Skrlatica is very wide and beautiful towards all sides. It matches the one from Triglav but in one aspect it is even better. From Skrlatica one can see something that is missing in Triglav panorama: the Father himself (as Slovenians call Triglav) and its monumental North face, which is from Skrlatica in full display.
Most direct and classic Skrlatica approach is from Vrata valley. It can be done in a day but you can count on leg muscle inflammation for next two days because of 3.5km of altitude difference! This combination requires long day. You can make it easier if you split the climb in two days by reaching the Rusje bivouac on the first day (afternoon).
Same goes for Krnica valley route and it is even tougher, longer and has bigger altitude difference which is over 4km! This route is almost undoable in both ways in a day. You can split it in two by descending to Rusje bivouac after the summit and tomorrow descent back to Krnica.
If it sounded tough for previous 2 routes Trenta valley route is even tougher than Krnica and has even bigger altitude difference. One has to be really crazy to do this route both ways in a day and it is impossible to complete it during the daylight but night descent from Pogacnikov Dok hut to Trenta valley is not a problem. Because of the position of Pogacnikov Dom hut it is not even easy to split this route in two days and have two easier days. When doing Trenta route it is best to do it in 3 days and combine with some of the nearby peaks like Razor (2601m), Planja (2447m), Pihavec (2414m), Kriz (2410) and Stenar (2501m).
Here is very beautiful two day combination from Vrata valley. On the first day (morning start) reach Pogacnikov Dom via Sovatna. In the afternoon climb Razor and sleep over. On the second day head towards Skrlatica via Dolkova Spica, which you will climb on the way because its summit is close above Rdeca Skrbina pass. From the summit of Skrlatica descent to Vrata valley via classic route.
Here is beautiful three day combination from Trenta valley. On the first day (morning start) reach Pogacnikov Dom. In the afternoon climb Razor and sleep over. On the second day head towards Skrlatica via Dolkova Spica, which you will climb on the way because its summit is close above Rdeca Skrbina pass. From the summit of Skrlatica return to Pogacnikov Dom via Rusje Bivouac and sleep over. On the third day, before descending back, climb nearby Pihavec or Stenar. Or even better, head via Luknja pass towards Triglav and extend your trip.
Best period to climb Skrlatica, if you don't like snow and extreme climbs, is from July to October. In June it is not cold anymore but there can be quite a lot of steep snow fields on the routes, which of course is not a problem for equipped mountaineer. Most beautiful time to visit in main season is October when golden larches shine on the slopes of Julian Alps, especially in second half of October. Also air is cleanest in October when comparing with other main season months.
Outside that period it is cold with lot of snow. Best route is from Vrata valley (Aljazev Dom hut) because it's least technical and shortest. Up to summit climb are non techical, but steep snowy slopes. Summit climb pegs and fixed ropes are under snow, which turns Skrlatica in unreachable ice fortress reserved only for experienced alpine climbers, which know to deal with such technical problems (up to IV grade).
Pogacnikov Dom hut route is also not technical till summit climb but is too long for short winter days. If you want to do it split climb in two days by sleeping in huts winter room.
Krnica valley route is only for experts in winter because of almost perpendicular, 300m high, ferratta section surmounting Kriska Stena face.
Snow is possible even in summer but it won't remain on ground before October. In summer significant is daily cloud development. From my experience and observations, Skrlatica is peak, which spends more time in the clouds than any other peak in Julian Alps.
Mountain conditions in Julian Alps are well known thanks to Kredarica (2515m) hut and meteo station, which is just below the Triglav (2864), highest peak of Julian Alps. Because Mojstrovka is some 200m lower than Kredarica temps are few degrees higher.
You can also observe current conditions and forecast for Kredarica on the Wunderground meteo site.
Current weather and forecasts can also be found on the Slovenian Environment Agency pages.
3 routes from 3 different valleys mean 3 different trailheads. How to reach them is described in each route section.
The heart of the region is Kranjska Gora resort town, 84 kilometers from the Slovenian capital Ljubljana. Mojstrana village, 13km before Kranjska Gora, when coming from Ljubljana, is center to visit Vrata valley.
If you want to reach Ljubljana, Slovenian capital, by plane check a timetable on the site of Adria Airways, a national airline.
From Ljubljana buses depart towards Mojstrana and Kranjska Gora every 60 minutes. During the season and when there is no snow buses connect Kranjska Gora with Bovec town. This line goes over the Vrsic pass and into the Trenta valley which takes you to Trenta valley trailhead.
In Mojstrana and Kranjska Gora direction, train will take you to Jesenice town, 10km before Mojstrana where you would have to wait for the bus from Ljubljana. Jesenice are on the main railway from Ljubljana towards Austria and Germany so it can be reached by train from Western Europe. See schedules on the sites of Slovenian railways and German railways.
From Ljubljana via the highway towards Karavanke tunnel and via the road it is 71km to Mojstrana and 84km to Kranjska Gora.
From central Europe approach leads through Villach, Austria: via Karavanke tunnel (around 40km) or Korensko Sedlo pass (around 30km).
From western Europe approach leads through Udine, Italy: exit from Udine – Villach highway in Tarvisio. From Tarvisio to Kranjska Gora is another 20km.
Aljazev Dom (1015m) (Aljaz Hut) is placed in upper part of Vrata valley, near the forest end. It is accessible by car, 12km from Mojstrana village, which lies on the main road from Ljubljana (72km) to Kranjska Gora resort (12km). It was opened in 1896. In 1909 the hut was destroyed by avalanche. New hut was opened the next year where it stands today. It has 150 beds and is open from beginning of May till the end of October. Winter room has 8 beds. Hut also has phone, electricity, warm water and so on. From the hut view is beautiful on the peaks around the valley, which rise wildly above it, and especially on Triglav and its North face.
Pogacnikov Dom na Kriskih Podih (2050m) (Pogacnikov Dom hut on Kriski Podi) is standing on the edge of Kriski Podi basin, high above the Trenta valley and is 'home' hut for Razor. Kriski Podi are bare rock basin, which is ascending in few steps. At the foothills of those steps lie 3 beautiful alpine lakes: lower, middle and upper Krisko jezero lakes. Area is surrounded from 3 sides by peak. Highest of them is Razor (2601m). The hut was opened in 1951 and named after a Joze Pogacnik whose idea was to build a hut here. Unfortunately he died on the way from Trenta valley to hut opening ceremony. In 1985, near the hut, load aerial ropeway and winter room were built. The hut is open from July 1st till the end of September. It has 67 beds + 16 in winter room, water and electricity from a generator. View from the hut is beautiful towards Trenta valley and Soca River, which shines on the afternoon sun and the wild peaks around.
Koca v Krnici (1113m) (Hut in krnica) stands on a small meadow in conifer forest on the bottom of Krnica valley. The valley is surrounded by high peaks: Skrlatica (2740m), Razor (2601m) and Prisojnik (2547m). Opening year was 1933. It is open from May 1st till October 31st, while outside that frame during weekends and holidays. It has 20 beds, water and power from a generator.
Bivak IV na Rusju (1980m) (Bivouac IV on Rusje) stands high above Vrata valley, on the slopes below Dolkova Spica (2591m) and Stenar (2501m), since 1948. During the 1950/51 winter it was blown away in the storm and ended up some 80 meters away. In 1953 a new one has been built. It is constantly open and has 10 sleeping places, furnace and water reservoir.
Skrlatica and its surroundings is in the Triglav National Park but there is no entrance fee. The only thing charged is parking on selected locations.
here is an interesting note about possible skiing from the summit of Skrlatica: Two well known Slovenian climbers, Marijana Cuderman & Marko Kern (see their famous page: Marijana & Marko) did on May 7th, 2006 this interesting route: From Vrata valley they ascended Skrlatica by the normal route (foggy, lousy weather), then they skied down from the summit into V Kotlu basin (45 degrees, IV, exposed in the upper part), crossed the basin, climbed on the notch between Visoki and Srednji Rokav, and finally skied down the couloir from the notch (45 degrees, III+, 200m) and further all the way into Vrata valley. Great tour!


Nipsey Hussle after soundcheck holding his original Antoinette Cauley piece at the Cluture show in Phoenix.
Futuristic holding his custom Antoinette Cauley painting. This piece is permanently on display at Guest List inside of Arizona Mills Mall in Tempe, AZ.
Antoinette being interviewed by the Phoenix Art Museum to promote Kehinde Wiley's: A New Republic. Antoinette ran life drawing workshops through the opening night of the exhibition. The museum broke a record for most people in attendance seeing a little over 7,000 people.


24 years old. Grew up North Coast NSW. Came to Armidale for uni. Bachelor of Arts (History). Keen to serve the church for the glory of God and the growth of his kingdom. Having been encouraged and grown significantly in my faith while a student through the work of a previous MTS'er, I hope to be able to serve others in the same way.
After attending St Mark's for five years as a university student, I've been incredibly blessed to become a ministry apprentice here. I hope to continue growing in Christian maturity and service over the course of my apprenticeship as a basis for long-term ministry going forward.
For growth and maturity in all aspects of the Christian life. That I would be captivated by the glory and urgency of the gospel. That the Lord would enable me to faithfully minister his word in one-to-one, bible study, and church contexts. That the team here would find an open door for the spread of the gospel.


text:
preprints.org > life sciences > biochemistry > doi: 10.20944/preprints201612.0044.v1
In Vitro and in Vivo Antiplasmodial Activity of Extracts from Polyalthia suaveolens, Uvaria angolensis and Monodora tenuifolia (Annonaceae)
Alvine N. Mfopa , Lauve R. Y. Tchokouaha , Cedric D.J. Mbouna , Marthe A. T. Tchuente , Rufin M. T. Kouipou , Patrick V. T. Fokou , Eugenie A. M. Kemgne , Raceline G. Kamkumo , Fabrice F. Boyom *
Version 1 : Received: 7 December 2016 / Approved: 8 December 2016 / Online: 8 December 2016 (08:59:49 CET)
How to cite: Mfopa, A.N.; Tchokouaha, L.R.Y.; Mbouna, C.D.; Tchuente, M.A.T.; Kouipou, R.M.T.; Fokou, P.V.T.; Kemgne, E.A.M.; Kamkumo, R.G.; Boyom, F.F. In Vitro and in Vivo Antiplasmodial Activity of Extracts from Polyalthia suaveolens, Uvaria angolensis and Monodora tenuifolia (Annonaceae). Preprints 2016, 2016120044 (doi: 10.20944/preprints201612.0044.v1). Mfopa, A.N.; Tchokouaha, L.R.Y.; Mbouna, C.D.; Tchuente, M.A.T.; Kouipou, R.M.T.; Fokou, P.V.T.; Kemgne, E.A.M.; Kamkumo, R.G.; Boyom, F.F. In Vitro and in Vivo Antiplasmodial Activity of Extracts from Polyalthia suaveolens, Uvaria angolensis and Monodora tenuifolia (Annonaceae). Preprints 2016, 2016120044 (doi: 10.20944/preprints201612.0044.v1).
Mfopa, A.N.; Tchokouaha, L.R.Y.; Mbouna, C.D.; Tchuente, M.A.T.; Kouipou, R.M.T.; Fokou, P.V.T.; Kemgne, E.A.M.; Kamkumo, R.G.; Boyom, F.F. In Vitro and in Vivo Antiplasmodial Activity of Extracts from Polyalthia suaveolens, Uvaria angolensis and Monodora tenuifolia (Annonaceae). Preprints 2016, 2016120044 (doi: 10.20944/preprints201612.0044.v1). Mfopa, A.N.; Tchokouaha, L.R.Y.; Mbouna, C.D.; Tchuente, M.A.T.; Kouipou, R.M.T.; Fokou, P.V.T.; Kemgne, E.A.M.; Kamkumo, R.G.; Boyom, F.F. In Vitro and in Vivo Antiplasmodial Activity of Extracts from Polyalthia suaveolens, Uvaria angolensis and Monodora tenuifolia (Annonaceae). Preprints 2016, 2016120044 (doi: 10.20944/preprints201612.0044.v1).
The present study aimed at investigating the in vitro and in vivo susceptibility of malaria parasites to crude extracts and fractions from Polyalthia suaveolens, Uvaria angolensis, and Monodora tenuifolia. The ethanolic extracts were prepared by maceration, and were further partitioned using water, dichloromethane, hexane, and methanol. The most promising fraction was subjected to column chromatography and the sub-fractions tested for activity in vitro. The antiplasmodial effect of extracts and fractions was tested against the Chloroquine resistant (PfK1) strain in 96 wells microtiter plate format using SYBR green florescence assay. The promising fraction was further assessed for cytotoxicity and acute toxicity in Swiss albino mice and subsequently against the rodent malaria parasite, P. berghei. Qualitative phytochemical screening was also performed on the promising fraction. The methanol fractions exerted the overall better effect with that of the twigs of P. suaveolens (PStw(Ace)) showing the highest potency with a IC50 value of 3.24 µg/mL followed by the fractions of leaf of M. tenuifolia (MoTel(Ace), IC50= 3.84 µg/ml) and stem bark of P. suaveolens (IC50= 4.90 µg/ml). The phytochemical screening showed the presence of alkaloids, lactones, and phenols in the more active fraction of P. suaveolens (PStw(Ace)). The chromatographic fractionation of this fraction led to 12 sub-fractions with PS8 sub-fraction being the most active (IC50= 4.42 µg/mL). In vivo, oral administration of 2000 mg/kg b.w of fraction PStw(Ace) in mice showed no signs of toxicity. Also, fraction PStw(Ace) at 400 mg/kg b.w exerted the highest suppressive effect against P. berghei strain B throughout the 4 days experiment (% parasitaemia below 5.2%). Overall, the results achieved supported the use of the three plants in the traditional treatment of malaria in Cameroon. More interestingly, the methanolic fraction of the twigs extract from P. suaveolens might be of interest in future development of an antimalarial phytodrug.
Polyalthia suaveolens; Uvaria angolensis; Monodora tenuifolia; Plasmodium falciparum K1; toxicity; antimalarial


It's a label soundclash ting ! Natty Dub Recordings are back to challenge the dog! The mighty CABIN FEVER DNB will be repping all things natty while in the red corner Ruffneck Ting will be firing out the ammo coutesy of Jinx, Dazee, K Jah and Vytol. Hang on a minute …Do we detect some double agent action? …In that case anything could happen…Plus Trafic, Ydott, Megatron and Deanie Rankin on hosting duties. Gonna be large! 9-4am at the Attic !