text:
Biografia

Il padre, Juan de Villagra, fu un ufficiale civile di importanza minore. Nel 1537 si spostò dalla Spagna a Cartagena de Indias, e da qui a Santa Marta ed in Perù. Giunse in Cile con la spedizione di Pedro de Valdivia.

Dopo la fondazione di Santiago, Villagra ricoprì per quattro anni la posizione di sindaco. Valdivia gli concesse anche un'encomienda a Tirúa. Dopo la morte del governatore, tornò in Perù dove sposò Beatriz de Figueroa.

Tornò di nuovo in Cile quando il nipote Francisco de Villagra era governatore per la prima volta. Combatté nella guerra di Arauco comandando le forze meridionali quando il governatore si ammalò. Nel 1556 era alla guida dei soldati che scacciarono Lautaro da Santiago, con la battaglia di Peteroa.

Era ancora comandante quando Francisco de Villagra divenne governatore per la seconda volta, nel 1561. Alla morte di Francisco de Villagra, il 22 giugno 1563, divenne governatore ad interim. Questo titolo fu in seguito confermato dal viceré del Perù, Diego López de Zúñiga. La sua strategia militare lo portò a concentrare le sue forze, abbandonando il forte di Arauco per poter potenziare Angol e Concepción. Alcune delle più dure sconfitte Mapuche furono causate dagli assalti ad Angol, dove la guarnigione guidata da Lorenzo Bernal del Mercado causò oltre mille morti, tra cui il toqui Illangulién, nella battaglia di Angol. In seguito guidò una nuova campagna nel sud, ponendo fine all'assedio di Concepción e riportando vittorie nelle battaglie di Reinohuelen e di Tolmillán, contro i Mapuche stanziati a nord del fiume Bío Bío. Questa serie di vittorie portò ad alcuni anni di apparente pace tra spagnoli e Mapuche.

Con la morte del viceré López de Zúñiga y Velasco nel 1564, la situazione politica peggiorò per Villagra. Nel 1565, per ordine del viceré Lope García de Castro, fu sostituito da Rodrigo de Quiroga, arrestato e mandato in Perù, dove riuscì a ripulire la sua fama. Dopo questa assoluzione chiese al re di ottenere i risarcimenti che era convinto di meritare, ma non ottenne mai risposta.

Morì a Lima l'11 settembre 1577.

Collegamenti esterni

Governatori Reali del Cile
Esploratori dell'America meridionale


With today's robust talent pool, resumes for open positions can coming flooding in, and you may not have time to read every one thoroughly.
Here are some tips from industry professionals on what to look for that can help you qualify candidates quickly and confidently.
It is so critical that a company's success or failure may be predicated on how well it practices these core values.


text:
using namespace std;

class NoSuchRuleStringException: public exception
{
public:
	NoSuchRuleStringException(const char* ruleString){
		this->ruleString = ruleString;
	}

	virtual const char* what() const throw(){
		return ruleString;
	}
private:
	const char* ruleString;
};

redpajama_set_name: RedPajamaGithub


text:
Airtel and Jio get into 5G sprint
Giants seek first mover advantage
/ By Shreyansh Mangla / New Delhi
Benefits and uptake of 5G mobile telephony services in India remain to be seen
Days after the official launch of 5G mobile telephony services in India, two of the biggest players, Reliance Jio and Airtel have gotten into the act, aggressively building for introducing the service as soon as possible, with the hope of capturing higher market share.
Last week as the 5G network was officially launched in India by Prime Minister Narendra Modi at the India Mobile Congress (IMC), two of the biggest players in telecom, market leader Reliance Jio and its closest rival Bharti Airtel announced their own plans to start rolling out the service across the country in phases, with the aim to extend their 5G footprint all over India in the shortest period of time.
However, the full rollout of the 5G services will take place in phases and will be first launched in 13 Indian cities, that include Ahmedabad, Bengaluru, Chandigarh, Chennai, Delhi, Gandhinagar, Gurugram, Hyderabad, Jamnagar, Kolkata, Lucknow, Mumbai and Pune.
The technology promises to not only bring a speedier network for a data-hungry generation, but will also lend a helping hand to some public service sectors, such as healthcare, on-farm technologies, and swift disaster management. The IMC has showcased opportunities emerging in the digital realm in 2022.
Standalone or Non-standalone
Mukesh Ambani's Reliance Jio will roll out in standalone mode, a slightly sluggish version of the 5G network but its 700 Mhz spectrum compensates for the loss. While its rival, Bharti Mittal-owned Airtel does not own a high spectrum bandwidth, it will roll out its 5G services in NSA (or Non-standalone mode), which offers better call quality to the users and more stable connections. While a standalone spectrum is built specifically for a 5G network, NSA has a 5G network built over a 4G network, which provides more stability and is a lot more affordable than standalone networks.
But Jio is going ahead with its standalone model as it aims to target high-end consumers with the launch of a 5G network across India, even though it is more expensive than Airtel's NSA network. However, the telecom business is full of surprises. When Airtel witnessed phenomenal growth during the lockdowns of 2020, Jio retaliated aggressively by boosting its OTT platforms. This led to both the firms getting locked into a neck-to-neck competition.
In 2021, Airtel revolutionised IoT technology in India when it noticed an important trend in the industry that stated that 20-30 pc of digital ads were completely ignored by the spectators. Therefore, Airtel decided to offer four brand new services on different platforms, including Airtel mobile network, Broadband and landline, DTH through Airtel TV, Airtel Thanks for online payments and Airtel Wynk Music.
In terms of data usage, there is not much to separate the users of the two telecom giants. Jio users consume about 12 to 14 GB of data per month, whereas Airtel users consume 16-20 GB of data a month. With its advertising services, Airtel may be able to generate more advertising revenues. Also, by going with NSA model, Airtel says its download speeds would be faster as it is possible to use 4G mid-band airwaves along with C-band 5G spectrum to obtain faster download speeds.
It is a noted trend in the business of telecom that once the users become habituated to a particular ecosystem, chances are they will use other services of that ecosystem as well. Airtel, through its Xstream app, demonstrated how it could hook users to its platforms. It introduced 170 OTT platforms on the app with the facility to download content for offline viewing. Initially, most of its services were free of charge, an offer that attracted even more users. Using these platforms, Airtel will generate revenue from more than 350 million users by showing them ads. Airtel shows six different types of ads to its users: Display ads, Video Ads, Audio ads, SMS ads, Call ads, and DTH ads. Although, Jio's ecosystem is much larger than Airtel's, that includes Jio telecom, broadband, LIVE TV, Jio Cinema, newspaper, money, and Saavn Music.
5G boost for many sectors
According to Ericsson's mobility report, 5G will not only benefit the rural population, but it will also give a boost to urban gamers, innovators across cloud computing, and cross-platform sharing, including the use of AI and VR technologies.
However, students at schools and universities in India look forward to using 5G mobile telephony in order to bridge the gap created by the digital divide. In a recent survey, conducted by Opensignal, asking people's opinions about which sector is going to get the maximum boost through the introduction of 5G technology, people voted for education as their preference.
"I believe that 5G is going to bring a dramatic change in all sectors, bridging the digital divide. If you look at the way data is consumed in the Indian market, it is all going to change for the better. So, even the education sector will be benefited. The way we do marketing, FMCG consumption, or banking, the way information is consumed, it's all going to change. With its extremely low latency rate, 5G will offer faster, more reliable and smoother content delivery to the students," Deepak Gupta, Principal Consultant at R K Swamy BBDO, a large advertising agency in New Delhi, tells Media India Group.
Many believe that Indian users have started using the internet productively since the onset of Covid-19 lockdowns. "Probably because of how most people in India consumed online content during the pandemic, people have started shifting their focus towards self-growth and finding new opportunities. Here, 5G is going to take them one step further," Shipra Raj, Researcher, Department of Media and Communication, Jamia Millia Islamia, tells Media India Group.
Moreover, by 2023, it is estimated that with the deployment of the 5G networks in India, brands will revolutionise the way they advertise their products and target their audience. Advertising will no longer remain a one-to-one medium. Customers and vendors will be able to send their videos to digital posters, where they can interact with each other. It is also rumoured that the audience can interact with the characters in the ads. As each person will see different ads based on his/her preference, brands will be able to target their audience better with the rollout of 5G services.
There are many reported features that the telecom providers highlight about the capabilities of 5G. These include digital billboards that will display real-time updates on local weather, news, speed limits or public announcements. The biggest advantage of digital billboards will be their fluidity. They will display real-time updates faster than the traditional billboards in India, where static text is displayed for weeks.
However, experts say that most of the demonstrated features of the 5G technology have already been introduced earlier, but only time will tell whether 5G can give it a boost or not. "The 3D hologram or VR technology has been demonstrated even before. Way back in 2014, even when Modi contested parliamentary elections, at that time he had used holographic images, that too in a live broadcast. He was delivering a speech in Delhi, and people could see his 3D figure through a live feed. I hope that this concept gets enhanced by the introduction of 5G technology," says Deepak Gupta of RK Swamy BBDO.
It may take some time to see how good the 5G technology may be. But one of the basic hurdles in 5G adoption nationwide is that very few consumers in India own 5G-enabled smartphones. And even then when a consumer is ready to surf on 5G, the higher cost of the plans may put them off. After all, the total number of mobile subscribers in India fell in 2021 December from 1.154 billion to 1145 billion and since then it has declined further to 1.01 billion in April 2022.
When 5G arrives in India, the cost of the data plans will increase surprisingly after the initial benefits. Chances are that these plans will soon become unaffordable to an average mid-segment consumer.

redpajama_set_name: RedPajamaCommonCrawl


text:
Reading: Spain's La Liga To Resume Season on June 8
Lifestyle Uganda > Blog > Lifestyle Uganda > Spain's La Liga To Resume Season on June 8
Lifestyle UgandaNewsSports
Spain's La Liga To Resume Season on June 8
Ssendaza Ismail
La Liga is free to resume. PHOTO/Shutterstock
Spain's Prime Minister Pedro Sanchez has confirmed that La Liga is free to resume from June 8.
In a speech on Saturday, he said, "The time has come to resume many daily activities." "La Liga will return from June 8. Spanish football has a huge following. Sources said that the target date for the restart of the 2019-20 season is June 12, with a specific date to be announced.
The derby match between Sevilla and Real Betis is expected to be the first game to restart the campaign. The 2019-20 La Liga season was declared a state of emergency on March 12.
Players were forced to practice at home until the gradual easing of the lockdown restrictions earlier this month. Initially, the Spanish 42 First and Second Division clubs were allowed individual exercises on the training ground before the group began training sessions, with up to 10 players in the week of May 18.
SEE ALSO Learn How to Care For Your Weave Hair Extensions
The next phase will be a full training session in which players can reflect on competitive situations and work on tactics for the first time.
La Liga has already sent an order to clubs detailing the safety measures for the tournament, which will take place without fans at the end of the season.
The successful opening of the German Bundesliga helped pave the way for other European football leagues. Whenever leagues in England and Italy return, expect a similar design to Spain – five substitutes per game, closed-door matches, masks and social distances when possible.
All of these will be the norm for the final stages of the Time19 -'20 campaign.
The league will resume with some interesting plays around the positions in the schedule. Barcelona (58 points) lead Real Madrid (56 points) by 2 points in 11 games. While no team will play each other again this year, there will be an impressive title match in Spain.
SEE ALSO New Tools From Bandlab: Zire and Crowd Review Raise Your Music's Profile
The race for the top four will have its fair share of drama. Sevilla is in third place with 47 points, Real Sociedad and Getafe are in 4th place with 46 points, Atletico Madrid in 6th place with 45 points and Valencia in 7th place with 42 points.
With all those teams focused on Champions League and Europa League, expect a lot of turnovers in the 3-7 rankings.
Football in Europe is slowly returning, which is indicative of the presence of better times.
Source: Lifestyleug.com
BRIT Awards 2023 nominated Burna Boy and Fireboy DML
TAGGED: derby between Sevilla Real Betis, derby match Sevilla and Real Betis, Getafe are in 4th place, La Liga free to resume, La Liga Season on June 8, La Liga To Resume on June 8, Real Sociedad in 4th place, Sevilla in third place, Spain's La Liga To Resume
Ssendaza Ismail 27th May 2020
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By Ssendaza Ismail
A Blogger that gives you the latest news and gossip on the hottest local and international celebrities. Previously, Ismail worked as a System Administrator at Pearl VoIP & 3GTelecommunication UK for 6 months as remote Network operations center engineer(NOC). Let's talk, WhatsApp: +256753659743
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Use the filter button at right to narrow down to product required or simply use search button at top to search for desired product. Go to "Home" to return to main page and category of products.
Our guarantee to you: We pick the freshest and highest quality of fresh vegetables and fruits for our customers. If upon delivery, you are unsatisfied with the quality of vegetables and fruits, we will exchange with no questions asked.


text:
Voitko kuulla äänen sen (Fins voor Kan je Zijn stem horen) is een compositie van Fridrich Bruk. Het werk bestaat uit een vijftal liederen op tekst van de Finse pastor/dichter Pirkko Arola (geboren 1946).

De vijftal religieuze liederen zijn:
 Isän syli (In de armen van de Heer) (voor zangstem, orgel)
 Tahdon olla (Ik wil zo graag)
 Voitko kuulla äänen sen (Kan je Zijn stem horen)
 Oi, Jeesus, rakkautesi (Oh Jezus, je liefde)
 Nousee ruohoon kukkanen (Een bloem groeit)

Of het totale werk ooit is uitgevoerd is niet bekend.

Lied (klassieke muziek)
Compositie van Fridrich Bruk
Compositie voltooid in 1984

redpajama_set_name: RedPajamaWikipedia


text:
CCRC refers conviction due to concerns about prosecution witness
Go back to News
#referrals
The Criminal Cases Review Commission ("CCRC") has today decided to refer Mr Uthayathas Balasubramaniam's 2004 conviction for conspiracy to commit assault occasioning actual bodily harm to the Court of Appeal, after new information came to light about a key prosecution witness.
On 6 November 2001 Sellathurai Balasingham was attacked and beaten to death by a group of men near to his home in South London. Mr Balasubramaniam was one of a number of men charged with his murder. Prior to his trial at the Old Bailey, one of Mr Balasubramaniam's co-defendants offered to plead guilty to a lesser offence and give evidence for the prosecution.
The prosecution case against Mr Balasubramaniam relied upon a version of events provided by this man, who became the principal prosecution witness. Before giving evidence at the trial, he disappeared and his statement was read to the jury under the "hearsay" provisions of the Criminal Justice Act 2003. The jury acquitted Mr Balasubramaniam of murder but convicted him of conspiracy to commit actual bodily harm. Mr Balasubramaniam unsuccessfully appealed against his conviction in 2010.
Following several appeals and re-trials, the Court of Appeal quashed the convictions of all but one of Mr Balasubramaniam's co-defendants in 2011. During those proceedings new information came to light, including an undisclosed "deal" with the prosecution, which called into question this witness's credibility.
The CCRC was contacted by Mr Balasubramaniam in April 2019. Following a detailed review of his case, the CCRC has decided that there is a real possibility that the Court of Appeal will now quash his conviction because this witness can no longer be regarded as credible.
CCRC Chairman Helen Pitcher said: "This case is a good example of why the CCRC is such an important part of our Criminal Justice System. New information has come to light, years after Mr Balasubramaniam's trial which now calls into the question the safety of his conviction. We've carried out a thorough, independent review of the case and decided that it needs to be looked at again by the Court of Appeal."
Mr Balasubramaniam is a Sri Lankan national who voluntarily returned to Sri Lanka in 2012 when his various applications for leave to remain in the UK were refused. There is a Home Office exclusion order against him preventing his return to the UK although his spouse is a UK resident.
The CCRC is also appealing for Mr Balasubramaniam's final co-defendant, Mr Kumarasritharan Mukundan, to come forward, so his case can be considered too.
Mr Balasubramaniam was represented by James Nicholls of Birds Solicitors Ltd in his application to the CCRC.
This press release was issued by the Communications Team, Criminal Cases Review Commission. They can be contacted by phone on 0121 232 0900 or by email press@ccrc.gov.uk.
The Criminal Cases Review Commission ("CCRC") is an independent body set up under the Criminal Appeal Act 1995. It is responsible for independently reviewing suspected and alleged miscarriages of criminal justice in England, Wales and Northern Ireland. It is based in Birmingham and is funded by the Ministry of Justice.
There are currently 11 Commissioners who bring to the CCRC considerable experience from a wide variety of backgrounds. Commissioners are appointed by the Queen on the recommendation of the Prime Minister in accordance with the Office for the Commissioner for Public Appointments' Code of Practice.
The CCRC usually receives around 1,400 applications for reviews (of convictions and/or sentences) each year. Since starting work in 1997, the CCRC has referred around 3% of applications to the appeal courts.
The CCRC considers whether, as a result of new evidence or argument, there is a real possibility that a conviction and/or sentence would not be upheld were a reference to be made. New evidence or argument is argument or evidence which has not been raised during the trial or on appeal.  Applicants should usually have appealed first. A case can be referred in the absence of new evidence or argument or an earlier appeal only if there are "exceptional circumstances".
If a case is referred, it is then for the appeal court to decide whether the conviction is unsafe or the sentence unfair.
More details about the role and work of the Criminal Cases Review Commission can be found at www.ccrc.gov.uk The CCRC can also be found on Twitter: @ccrcupdate and Instagram: the_ccrc


For Congress, things seem to be out of control in four out of five constituencies.
BENGALURU: The Congress that is gung-ho about taking on Prime Minister Narendra Modi in the 2019 general elections seems to have lost the November 3 by-poll battle even before it has started. The party's struggle to finalise its candidates and discontent in its ranks indicate that it is not battle-ready.
For Congress, things seem to be out of control in four out of five constituencies. While the party is still unable to identify strong candidates in Ballari and Shivamogga Lok Sabha seats, it has not been able to contain dissidence in Mandya Lok Sabha and Ramanagara Assembly segments where its coalition partner JD(S) is fielding its candidates. Jamkhandi Assembly constituency is the only solace and even here, it is banking on a sympathy wave for Anand Nyamagouda to save it from defeat.
"Indiscipline and last-minute preparations are not new to Congress, but current developments have exposed the tussle between different groups within the party," political analyst Mohan Ram said. "They lost the spirit to fight and it takes a long time to regain it," he said referring to a lack of strong candidates in Ballari and Shivamogga.
While the top leaders in the state are trying to convince the party MLAs from Ballari to put up a united front, the party seems to have surrendered Shivamogga LS seat to JD(S) as it could not identify a strong candidate to take on Yeddyurappa's son B Y Raghavendra. The real battle here is likely to be between JD(S) and BJP if JD(S) can convince former MLA Madhu Bangarappa to contest. Congress is yet to take a final decision.
Developments in Mandya and Ramanagara are also ominous for the coalition. The party is facing dissidence in Ramanagara and Mandya as it has not prepared its leaders to go to elections alongside JD(S). The local leaders have openly defied the high command's instructions to work for JD(S) candidates and some of them have even quit the party. In Ramanagara, Congress leader Iqbal Hussain has threatened to contest as an independent candidate. Such a move will be a big embarrassment for the party, though it may not have much of an impact on the outcome of the elections.
The developments in the last one week have exposed a lack of a coherent game-plan and strategy to channelise strength of its workers and expand their base. At the heart of all the confusion is the fact that no one knows who is in charge of the party affairs in Karnataka. Siddaramaiah is Congress Legislative Party (CLP) chairman, G Parameshwara is the Deputy Chief Minister, while Dinesh Gundu Rao is the KPCC chief.
Every time there is a crisis in the party, they all look up to the high command to resolve it. So much so that even for a decision like finalising two candidates for the by-polls, they had to approach AICC chief Rahul Gandhi. Congress' inability to put its act together may give greater leverage to JD(S) and increase its bargaining power when the parties sit for negotiations ahead of 2019 LS polls.


So you have decided to have a party, and have at least twenty mates descending on your place. How are you going to feed them? Ask everyone to bring a plate? That might work for your Nanna, but you're not so much into casseroles, and think of all those dishes. A BBQ might work? Except you don't have a BBQ and half your friends are vegetarian. Home delivery pizza? Maybe, except you want the party to go all night and don't want cold pizza left congealing on your kitchen table.
How about all-you-can-eat, made-to-order, fresh, hot wood fired pizza, cooked at your place? Oh, and starters and dessert pizzas?
Bella Pitsa, owned by Kath and Rossi, offer a mobile wood-fired pizza oven, complete with a chef who makes all the pizzas on-site with fresh West Australian ingredients. Only the pizza base is made in advance.
It was a cold July night when 40 guests arrived to celebrate a friend's 50th birthday. Knowing that there was plenty to celebrate and the party could go all night, the hostess had done her research, and decided that for the cost of eight small 'finger foods' from catering companies, she could get as much fresh pizza as her guests could consume.
Operating on an all-you-can-eat basis, Rossi will keep making and cooking pizzas until everyone declares they are full and can't eat another bite. And then he will make you dessert pizzas.
Although there was a mix-up with starting times, the mobile pizza oven – which was built by hand by Rossi – is kept burning, so it wasn't long before hot entrees were coming out to party guests. Small cups of Thai pumpkin soup, garlic bread, bruschetta and chicken and asparagus 'cups' kept guests happy while the pizzas were prepared.
A range of pizzas were offered including plain cheese and tomato for the kids, garlic prawn, potato and rosemary, Hawaiian, a very hot spicy seafood, and mushroom and feta. They offer a number of vegetarian options and can also provide gluten free bases on request. If you have a special request or a favourite topping, nothing seems to be too much trouble.
Although the crust was a little burnt at times (difficult to avoid considering the heat of the oven and the fact that the ultimate cooking time is only two minutes) the pizzas were fresh, hot and satisfying. They are not the ultimate in gourmet pizzas, nor are they over-loaded with heaps of toppings, but they are plentiful and fresh and pleased a wide range of palates.
After everyone had plenty to eat, and another half dozen pizzas were made to help the late night partiers soak up their chardonnay, three types of dessert pizzas were then brought out. The lemon meringue was the winner as far as I was concerned, and it amazes me that I had never seen it before. A layer of tart lemon spread on a plain pizza based, was then topped off with a layer of sweet meringue. The heat of the oven blackened it perfectly. I didn't get to try the caramel and Mars Bar pizza, which is probably for the best as I may not have been able to control myself, but I did try the apple crumble pizza, and would have liked to see apple slices rather than the purée we had on the night.
The price (per head) includes chefs, paper plates, serviettes, clean up and all the pizza you can eat. As each party is different and has unique requirements, prices may vary, but for the 40-50 guests at this particular party, the cost all up was $900. This averaged out to $20 a head, including starters, pizza and dessert, my friend didn't have to do any cooking and there was no cleaning up or dishes the next morning.
Bella Pitsa can do any weather, as they can bring their own waterproof canopy to work under, but it is important to remember the space required for not only the pizza oven (on a custom-built trailer) but the 4WD that pulls it along. It's probably not appropriate for someone planning to have a shindig on their 4th floor balcony. They also need access to a power point.
All party bookings made before October 10th (2012) will include free starters and dessert pizzas.
Thanks for this, it sounds like a real winner. The desert pizzas are calling to me...must find an excuse for a party!
Sounds so tasty, Shannon. A lovely read and your description of the dessert pizzas has me hungry!!
I am seriously salivating! Looks & sounds delicious! What a unique concept! Makes sense...Pizza to go without delivery woes!


text:
Q: Defining an array globally but its parameters will available later I want to use an array from a function HashTableInit to printHash. So, I defined it globally. But array's parameters are present in function HashTableInit. I don't want to take array by returning the function, because to use return I will need to call the whole function in printHash, and it will disturb my whole code.
void HashTableInit(int TableSize, int Key) {
//Create a space for HashTable as given in variable TableSize
struct hashTableNode * HT[TableSize];
for (int i = 0; i < TableSize; i++) {
    HT[i] = (struct hashTableNode*) malloc(sizeof (struct hashTableNode));
    HT[i] ->Key = 0;
    HT[i] ->next = NULL;
}

Here, TableSize will be available after this function executes. But how could I define array globally with parameters.

A: If it's not a pointer you can declare the variable with values with globally.
But in your case, it's a pointer variable. You have to manually allocate address before assigning the value. So it's a good practice to create a function to allocate values to the pointer variables. But you can assign the array and a variable to store the array size globally.I hope it will help you.

redpajama_set_name: RedPajamaStackExchange


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These delicious Zesty Lemon Macarons are filled with an easy to make lemon ganache and lemon curd. They are melt-in-your-mouth lemony good.
Heat 1/3 cup fresh lemon juice in a small non-reactive saucepan on medium heat to hot, but do not boil. Whisk 2 eggs, 1/2 cup sugar and 2 tsp. lemon zest in a medium bowl. Slowly pour hot lemon juice into egg-sugar mixture whisking constantly, then return mixture to saucepan. Cook over medium heat, stirring constantly with a wooden spoon, until mixture registers 170 degrees on instant-read thermometer and is thick enough to cling to spoon, about 3 minutes. Immediately remove pan from heat and stir in butter and lemon yogurt until smooth. Pour curd through fine-mesh strainer into a small bowl. Cover with plastic wrap directly on curd; refrigerate until cooled and ready to pipe onto Macarons.
In a medium bowl, whisk together powdered sugar and almond flour until blended. Sift almond flour mixture through a sieve into a medium bowl. If there is only a pinch of large chunks remaining, toss them out. In a mixing bowl with a whisk attachment, beat egg whites at medium speed until frothy; add cream of tartar, Whip until egg whites start leaving a trail; add castor sugar 1/3 at a time. Whip until stiff peaks form (when you pull out the whisk the peak should be stiff and not droopy, and you can hold the bowl upside down and nothing comes out.). Add 2 tsp. lemon zest, 1 tsp. fresh lemon juice, and yellow food coloring during the last minute of whipping. Add the flour mixture, 1/3 at a time, into the egg whites and gently fold in until fully incorporated (do not over mix, it should be like thick lava, and you can make a figure eight).
Prepare a template of 1-1/2″ circles about 2-inches apart (about 20 to a baking sheet 5 across by 4 down). Put the template under parchment on baking sheet. Fit a 16″ pastry bag with a 1/2-inch round tip (#1A tip) and fill the bag with the batter. Using the template as a guide, pipe circles onto the parchment papers. The peaks in the center should fall, if they don't wet your finger and pat the peak down. Tap the bottom of each sheet on the work surface, 4-5 times, to release trapped air bubbles. Let the cookies stand at room temperature for 30-60 minutes,to allow the cookies to develop their crusts. While the cookies are standing at room temperature, preheat oven to 320 degrees F. Once the cookies are dry to the touch, bake, one cookie sheet at a time, at 320 degrees F. for 13-15 minutes, until the top is not wiggly (error on the side of overcooked). Cool slightly, remove from parchment (they should release, if not, use an offset spatula) Let cool completely.
I tried this recipe after many and it was PERFECT! Thanks so much for sharing.
I'm glad you like them, thank you.


text:
\section{Turning-on the source\label{turning-on}}

Following  the recent realization of an atom laser in a waveguide \cite{Guerin06},
we shall consider the dynamics of matter waves with momentum $\hbar k_0$
released in a waveguide of frequency $\omega_{\perp}$,
tight enough so that the transverse excitation quanta $\hbar\omega_{\perp}$
is much larger than any other relevant energy scales.
Under such assumption, the radial degrees of freedom, being frozen, play no role and the system
becomes effectively one dimensional.
Moreover if the setup is horizontal, the gravitational field is constant,
avoiding the decrement of the de Broglie wavelength $\lambda_{dB}=2\pi/k_0$
due to the downward acceleration observed in vertical setups \cite{Guerin06}.
However, the effects of an arbitrary time-dependent linear potential,
of interest to achieve controlled transport, can be included following \cite{DM06a}.

The time evolution along the longitudinal axis can be tackled using
``source'' boundary conditions of the form
\begin{equation}\label{source0}
\psi(x=0,t)=\chi(t)\,e^{-i\omega_0 t}, \qquad \forall t>0,
\end{equation}
where the ``carrier'' frequency is related to the characteristic wavenumber of the beam by $\omega_0=\hbar k_0^2/2m$,
and the aperture function $\chi(t)$ modulates the wave amplitude
at the source. Such localized sources \cite{BT98,MB00} have been used for understanding tunneling
dynamics and related time quantities such as the tunneling times \cite{MSE02}, transient
effects in neutron optics \cite{GG84,FGG88,HFGGGW98}, and diffraction of atoms both in
time and space domains \cite{BZ97,DM05}.
The connection and equivalence between ``source'' boundary conditions,
in which the state is specified at a single point at all times and the usual initial value problems,
in which the state is specified  for all points at a single time, was studied in \cite{BEM01}.

Whenever the modulation of the source is sudden
($\chi(t)=\Theta(t)$, where $\Theta(t)$ is the Heaviside step function)
the resulting dynamics exhibits a wiggly density profile that, by analogy with the
diffraction of light from a semi-infinite plane, became known as
diffraction in time \cite{Moshinsky52,Moshinsky76}.
\begin{figure}
\begin{center}
\includegraphics[height=6cm,angle=0]{fig1.eps}
\caption{\label{sit}
Schematic snapshot of a suddenly turned-on atom beam propagating rightwards along a waveguide and exhibiting diffraction in time.
The wavefront of the density profile (d.p.) develops a set of oscillations, which is the hallmark feature of  diffraction in time,
in contrast with the uniform classical case.
Whenever the harmonic transverse confinement V is tight enough (represented by the concave sheet), the radial degrees of freedom are frozen out and the dynamics becomes essentially one dimensional, along the longitudinal axis $x$.
}
\end{center}
\end{figure}
Figure \ref{sit} shows a snapshot of the density profile of a suddenly turned-on atom beam,  with the oscillatory pattern
which is the tale-telling sign of diffraction in time.
This singular matter wave phenomenon has been observed in a wide variety of systems including ultracold neutrons
\cite{HFGGGW98} and atoms \cite{atomdit}, electrons \cite{Lindner05}, and even Bose-Einstein
condensates \cite{CMPL05}. Such experimental flurry together with the simplicity of Moshinsky's result has spurred a
series of works dealing with more complex setups \cite{Kleber94,MB00,GM05,DM05,DM06a}.

Here, instead of sudden switching we shall consider smooth aperture functions,
i.e., ``apodization'', a technique well-known in Fourier optics to avoid the diffraction effect
at the expense of broadening the energy distribution \cite{Fowles68}.
Manifold applications of this technique have also been found in time filters for signal analysis \cite{BT59}.

\section{Smooth switching: apodization and diffraction in time}\label{switching}

In this section we shall study the modification of matter-wave dynamics for slow aperture functions
with a finite switching time $\tau$. We introduce the continuous switching function
\begin{displaymath}
\label{switch}
\chi^{s}(t)=
\cases{
 0, \qquad t<0\\
\chi(t), \quad 0\leq t<\tau\\
1, \qquad t\geq\tau},
\end{displaymath}
where the superscript $s$ denotes that the source remain open for all $t>0$ (a {\it s}witch).
The family for which $\chi(t)=\sin^n\Omega_s t$ with $n=0,1,2$ and $\Omega_s=\pi/2\tau$ was considered in \cite{DMM07},
where it was shown that for fixed $\tau$, the apodization of the beam increases with the smoothness of $\chi(t)$,
this is, with $n$. Note that for $n=0$, one recovers the sudden aperture $\chi_0(t)=\Theta(t)$ which
maximizes the diffraction-in-time fringes. We shall consider a sine-square modulation in what follows ($n=2$)
and concentrate on the dependence on $\tau$.

\begin{figure}
\begin{center}
\includegraphics[width=7.5cm,angle=0]{fig2.eps}
\caption{\label{apodization}
Apodization in time. Removal of the sudden approximation in the switch of a matter wave
source leads to the suppression of oscillations in the beam profile characteristic of the diffraction in time.
The $^{87}$Rb beam profile is shown at $t=20$ms, and $\hbar k_0/m=1$cm/s.
For increasing $\tau$ the amplitude of the oscillations diminishes and the signal is delayed.
}
\end{center}
\end{figure}

Increasing the switching time $\tau$  leads to an apodization of the oscillatory pattern. As a result
the fringes of the beam profile are washed out, see Fig. \ref{apodization}.
In this sense, the effect is tantamount to that of a finite band-width source \cite{MB00},
and indeed this is the key to apodization, the suppression of diffraction is achieved broadening
 the energy distribution \cite{BT59,Fowles68}.
It is also analogous to the suppression of the current transients in
tunneling through a time-dependent barrier. Whenever the modulation of the potential is slow enough,
the resulting dynamics becomes adiabatic and the tunneling current tends
to the quasistatic equilibrium current \cite{SK88}.

However, the apodization lasts only for a finite time
after which a {\it revival} of the diffraction in time occurs, as shown in Fig. \ref{revival}.
The intuitive explanation is that the intensity of the signal from the apodization ``cap'',
see Fig. \ref{cap}, decays with time whereas the intensity of the main
signal (coming from the step excitation) remains constant.
For sufficiently large times, the main signal, carrying its
diffraction-in-time phenomenon, overwhelms the effect of the
small cap.
Indeed, from the linearity of the Schr\"odinger equation,
it follows that the wavefunction is the sum of a ``half-pulse'' term
associated with the switch released during the interval $[0,\tau]$ and a semi-infinite beam
suddenly turned on at time $t=\tau$.
\begin{figure}
\begin{center}
\includegraphics[width=7.5cm,angle=0]{fig3.eps}
\caption{\label{revival}
Revival of the diffraction in time.
During the time evolution of an apodized source, there is a revival of the diffraction
in time in the time scale $t_r=\omega_0\tau^2$ ($\tau=1$ms, $\hbar k_0/m=0.5$cm/s,
and $t_r=16.8$ms for a $^{87}$Rb source which is switched on following a sine-square function).
}
\end{center}
\end{figure}

One can estimate the revival time by considering the
momentum width induced by the apodization
cap, $\Delta p\approx
\sqrt{2m\hbar(\omega_0+\Omega_s)}-\sqrt{2m\hbar(\omega_0-\Omega_s)}
\approx\sqrt{2m\hbar\omega_0}\frac{\pi}{2\omega_0\tau}$,
and ballistic spread of the cap half-pulse
(we have checked numerically
that the classical dispersion relation for such pulse $\Delta x(t)\simeq\Delta x(0)+\Delta pt_r/m$ holds).
\begin{figure}
\begin{center}
\includegraphics[height=6cm,angle=0]{fig4.eps}
\caption{\label{cap}
Switching aperture function decomposition. In a switching process the aperture
function has a finite transient component
responsible for the apodization (filled area).
Such apodization cap is followed by a step excitation for $t\geq\tau$  (shaded area)
which leads eventually to the revival of diffraction in time.
}
\end{center}
\end{figure}

The ratio of the spatial widths corresponding to the initial
and evolved cap $\psi_{\chi}^{(1)}$ is given by
\begin{equation}
R=\frac{\Delta x(0)}{\Delta x(t_r)}\approx\frac{\Delta x(0)}{\Delta x(0)+\Delta pt_r/m}.
\end{equation}
Taking $\Delta x(0)=\sqrt{2\hbar\omega_0/m}\tau$ and imposing $R=1/2$ leads to
the expression for a revival time scale
\begin{equation}
t_r\approx \omega_0\tau^2,
\end{equation}
which is analogous to the Rayleigh distance of classical diffraction theory
but in the time domain \cite{Brooker03}.
The smoothing effect of the apodizing cap
cannot hold for times much longer than $t_r$.
This is shown in Fig. \ref{revival}, where the initially
apodized beam profile develops eventually spatial fringes, which reach the maximum value associated
with the sudden switching at $t\approx 2t_r$.

\section{Multiple pulses}\label{mp}

The matter-wave dynamics of a single pulse obtained from a source by means of
an aperture function $\chi^{(1)}(t)$ has been described in \cite{DM05,DMM07}
(hereafter, the superscript denotes the number of pulses in the aperture function).
Both the aperture function $\chi^{(1)}(t)$, and time-dependent wavefunction of
the associated pulse $\psi^{(1)}(x,t)$, allow a simple description of
matter wave sources periodically modulated in time.

More precisely, the $N$-pulse aperture function $\chi^{(N)}$ can be written as a convolution of
$\chi^{(1)}(t)$ with a grating function $g(t)$.
If the grating function $g(t)$ is chosen to be a finite Dirac comb
 $g(t)=\sum_{j=0}^{N-1}\delta(t-j T)$, it follows that
\begin{equation}
\chi^{(N)}(t)=\chi^{(1)}(t)*g(t)=\int dt'\chi^{(1)}(t-t')g(t')=\sum_{j=0}^{N-1}\chi^{(1)}(t-jT).
\end{equation}
Such modulation describes the formation of $N$ consecutive $\chi^{(1)}$-pulses,
each of them of duration $\tau$ and with an ``emission rate'' (number of pulses per unit time) $1/T$.

This mathematical framework can be employed to describe an atom laser
in the non-interaction limit. The experimental prescription for an atom laser
depends on the out-coupling mechanism.
Here we shall focus on the scheme described in \cite{Phillips99,Phillips00}.
The pulses are obtained from a condensate trapped in a MOT, and a well-defined momentum is
imparted on each of them at the instant of their creation through a
stimulated Raman process. The result is that each of the pulses  $\psi^{(1)}$
does not have a memory phase, the wavefunction describing the coherent atom laser being then
\begin{equation}
\phi^{(N)}(x,k_0,t)=\sum_{j=0}^{N-1}\psi^{(1)}(x,k_0,t-jT;\tau)
\Theta(t-jT).
\end{equation}
The Heaviside function $\Theta(t-jT)$ implies that the $j$-th
 pulse starts to emerge only after $jT$. It is interesting to impose a
relation between the out-coupling period $T$ and
the kinetic energy imparted to each pulse $\hbar\omega_0$, such that $\omega_0 T=l\pi$,
where if $l$ is chosen an even (odd) integer
the interference in the beam profile $|\phi^{(N)}|^2$
is constructive (destructive).

The diffraction in time is a coherent quantum dynamical effect,
we may expect it to be affected by noise in the environment.
If the phases between different pulses are allowed to fluctuate, the
interference pattern is affected \cite{VVDHR06}.
Moreover, if there is no phase coherence between different pulses,
the resulting density profile is the incoherent sum
of the single-pulse densities,
$\rho(x,t)=\sum_{j}\vert\psi^{(1)}(x,k_0,t-jT;\tau)\vert^{2}\Theta(t-jT)$,
which we shall use as a reference case.

One advantage of employing stimulated Raman pulses is that any desired fraction of atoms
can be extracted from the condensate. Let us define $s$ as the number of atoms out-coupled
in a single pulse, $\psi^{(1)}$. The total norm for the $N$-pulse incoherent atom laser is simply $\mathcal{N}_{inc}=sN$.
A remarkable fact for coherent sources is that the total number of atoms $\mathcal{N}_c$
out-coupled from the Bose-Einstein condensate reservoir depends on the nature of the interference \cite{Felipe}.
Therefore, in Fig.  \ref{atltime} we shall consider the signal relative to the incoherent case,
namely, $|\phi^{N}(x,t)|^2/\mathcal{N}_{inc}$.

\begin{figure}
\begin{center}
\includegraphics[height=6cm,angle=0]{fig5.eps}
\hspace*{.2cm}
\caption{
\label{atltime}
Time evolution of the density profile of a $^{23}$Na atom laser beam modulated by a sine-square function
with $\tau=0.833$ms, $T=0.05$ms, moving at $3.73$cm/s in the a) coherently constructive, b) incoherent case.
Note that $x_{cl}=\hbar k_0 t/m$ is the classical trajectory. In all cases the norm is relative to the
incoherent case, as explained in the text. The revival time is $174.4$ ms.
}
\end{center}
\end{figure}
Note the difference in the time evolution between coherently
constructive and incoherent beams in Fig. \ref{atltime}.
At short times both present a desirable saturation in the probability density of the beam.
However, in the former case a revival of the diffraction in time phenomena takes place in a
time scale $\omega_0\tau^{2}$, similar to the smooth switching considered in section \ref{switching},
whereas the later develops a bell-shape profile.

\section{Revival of the diffraction in time in an atom laser}

In an atom laser, the revival time can be related to the frequency of the BEC reservoir trap $\omega_{trap}$,
which determines the width of the out-coupled pulses.

First we note that whenever the overlap amongst different pulses
is coherently constructive or with phase memory (as in the periodic chopping of a beam),
an effective single-pulse aperture function can be introduced.
Indeed, if $\tau/T\gg1$ as in the actual experiments \cite{Phillips99,Phillips00},
it follows that an effective single-pulse aperture function of duration $\tau_{eff}=(N-1)T+\tau$ can be introduced,
 with a plateau in the time interval $[\tau,NT-\tau]$ and both a front and a back cap of duration $\tau$ associated with the switching on and off.
These caps determine the revival time $\omega_0\tau^{2}$.

Assume that atoms are out-coupled from the $n$-th longitudinal mode of the reservoir trap, whose
spatial width is $\xi_n=[(n+1/2)\hbar/m\omega_{trap}]^{1/2}$. Using $\omega_0=\hbar k_{0}^2/2m$,
and the semiclassical relation $\tau_n=m\xi_n/\hbar k_0$,
the revival time becomes
\begin{eqnarray}
t_r^{(n)}=\left(n+\frac{1}{2}\right)\frac{1}{2\omega_{trap}}.
\end{eqnarray}
A non-interacting Bose-Einstein condensate, one can take $n=0$.
This is a remarkable relation which states that diffraction in time manifest
itself since the beginning of the experiment in the limit of very tight traps which lead to narrow pulses.
However, if the Bose-Einstein condensate trap is broad,
so will be the out-coupled pulses and apodization will suppress the oscillations
on the density profile for times smaller than the revival time.

\section{Discussion}

We have studied the dynamics of non-interacting boson sources which are
modulated in time with an arbitrary aperture function.
Whenever the modulation is sudden, the spreading of the source exhibits an
oscillatory pattern in the density profile, which is the tale-telling sign
of the quantum diffraction in time phenomenon.
For smooth aperture functions the oscillations
are suppressed, thus bringing to the quantum domain the classical apodization techniques
usual in signal analysis and Fourier optics.
However, for long or multiple overlapping pulses
the smoothing is limited by a time scale $t_r$, associated with a revival
of the diffraction-in-time phenomenon.
Multiple pulse formation has been examined for different possible cases.
For constructive or for random averaged phases, a saturation effect occurs
providing a flat intensity profile before $t_r$, which later  develops
spatial fringes and a bell-shape profile respectively.

Though our results consider the dynamics under strong transverse confinement,
they can be extended beyond one dimension. Indeed, the effect of the dimensionality
on the diffraction in time phenomenon, have already been considered in a different context,
namely, the expansion of a single particle from cylindrical and spherical traps
\cite{Godoy03,Godoy05}. The result is that the amplitude of the oscillations decreases
in two and three dimensional setups in comparison with the dynamics along a tight-waveguide presented here.

Finally, we have restricted this work to the case of non-interacting bosons.
However, the presence of interactions between the out-coupled atoms
is expected to reduce the amplitude of the diffraction in time phenomenon,
as suggested by previous studies of quantum transients in the strongly interacting regime \cite{DM06}.

\begin{acknowledgments}
A. C. acknowledges the hospitality of the members of IF-UNAM during the completion of this work and financial support by the Basque Government (BFI04.479). The work has been supported by CONACYT (40527F), Ministerio de Educaci\'on y Ciencia (BFM2003-01003, FIS2005-01369 and FIS2006-10268-C03-01), and UPV-EHU (00039.310-15968/2004).
\end{acknowledgments}

\section*{References}

redpajama_set_name: RedPajamaArXiv


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text:
namespace Microsoft.Azure.Management.WebSites.Models
{
    using System;
    using System.Linq;
    using System.Collections.Generic;
    using Newtonsoft.Json;
    using Microsoft.Rest;
    using Microsoft.Rest.Serialization;
    using Microsoft.Rest.Azure;

    /// <summary>
    /// Http logs configuration
    /// </summary>
    public partial class HttpLogsConfig
    {
        /// <summary>
        /// Initializes a new instance of the HttpLogsConfig class.
        /// </summary>
        public HttpLogsConfig() { }

        /// <summary>
        /// Initializes a new instance of the HttpLogsConfig class.
        /// </summary>
        public HttpLogsConfig(FileSystemHttpLogsConfig fileSystem = default(FileSystemHttpLogsConfig), AzureBlobStorageHttpLogsConfig azureBlobStorage = default(AzureBlobStorageHttpLogsConfig))
        {
            FileSystem = fileSystem;
            AzureBlobStorage = azureBlobStorage;
        }

        /// <summary>
        /// Http logs to file system configuration
        /// </summary>
        [JsonProperty(PropertyName = "fileSystem")]
        public FileSystemHttpLogsConfig FileSystem { get; set; }

        /// <summary>
        /// Http logs to azure blob storage configuration
        /// </summary>
        [JsonProperty(PropertyName = "azureBlobStorage")]
        public AzureBlobStorageHttpLogsConfig AzureBlobStorage { get; set; }

    }
}


text:
\section{Introduction}

The Anderson transition\cite{anderson58,thouless74}, in which
eigenstates of non-interacting electrons are localized by disorder, has
long been a paradigm of a metal-insulator transition in solid state
physics.  The metallic phase  occurs only in three dimensions, since any amount
of randomness localizes all particles in one or two dimensions. In three
dimensions, a mobility edge separates localized states whose energies
lie at the edges of the spectrum, from extended states whose energies
lie in the middle.  The mobility edges appear for a
critical value of the disorder and move with the disorder until no
extended states remain. If the Fermi energy is located below or above
the mobility edge, inside the localized states, the system is then an
insulator.  Recently, research on this subject has experienced renewed
interest as localization of cold atoms in the presence of a disordered
optical potential has been observed \cite{aspect08, inguscio08}. Whereas
experiments in solid state physics are intrinsically limited as
interactions between electrons cannot be neglected, cold atoms allow the
exploration of the non-interacting regimes with possibilities of control
that could not be achieved before.

Another, simpler origin for an insulating behavior in a solid is the
presence of gaps due to a periodic potential applied to the particles.
These two possible insulating phases are in competition with each other
as they are based on opposite behaviors.  The Anderson insulator is due
to the localized nature of the wave function, whereas the gapped
insulator is due to its extended nature.  A third source of insulating
behavior is interactions between particles.  In many ways this is the
most difficult situation, since it involves treating the many-body
problem accurately.  In the systems with both interactions and
randomness, competition between Mott and band insulating phases have
been shown to result in metallic phases, as the two sources of
insulating behavior  counteract each other \cite{paris07,bouadim07}.
The possibility of metallic phases arising due to the addition of
interactions to two dimensional disordered systems has also been an area
of great interest \cite{abrahams79,lee85,belitz94}.

The goal of this article is to study the interplay between the two
sources of single particle insulating behavior- disorder and gaps
due to a periodic potential- in the context of non-Hermitian
matrices.  For this we
will use a modified version of the Hatano-Nelson model (HNM), that
includes at the same time a periodic potential that generates gaps in the
eigenspectrum and a disordered potential that will drive a localization
transition.  The HNM \cite{hatano96, hatano97} is a single particle,
random, non-Hermitian Hamiltonian that was introduced to study the
motion of magnetic flux lines in disordered type II superconductors, the
path integral representation of the HNM being analogous to a
classical model used to describe the flux lines. The HNM shows a
localization transition in one
dimension\cite{hatano96,hatano97,hatano98, feinberg99}. It is then a
very convenient tool to study the localization transition numerically,
as it allows the study of systems with large linear sizes.

The paper is organised as follows. In
the Sec.~II we introduce the HNM and recall some basic properties.
In Sec.~III, we present the different regimes which can be
observed.  Sec.~IV contains a detailed analysis of some
of the transitions appearing in the generalized HNM.
The conclusion describes some of the connections the additional term we
introduce into the Hatano-Nelson model has with the eigenspectrum of
several physical systems for whose properties random matrices have
been used.

\section{Modified Hatano-Nelson model}

\subsection{Hatano-Nelson model}
The Hatano-Nelson model is a discrete model similar to the Anderson
model used to study localization. In one dimension,
\begin{equation}
\mathcal{H}_{\rm HN} =\sum_{x=1}^L  \left[-\frac{t}{2}
\left( e^h c^\dagger_{x+1} c^{\phantom{\dagger}}_x
+ e^{-h} c^\dagger_{x} c^{\phantom{\dagger}}_{x+1} \right)
 + \mu_x n_x  \right]
\label{eq:ham}
\end{equation}
Here $c^\dagger_x (c^{\phantom{\dagger}}_x)$ are the usual fermionic
creation (destruction) operators and $n_x = c^\dagger_x
c^{\phantom{\dagger}}_x$ is the number of particles on site $x$.  The
first term of the Hamiltonian describes the hopping of particles between
sites, and the parameter $h$ controls the asymmetry between the hopping
amplitudes in the left and right directions.  We will choose the
random sites energies
$\mu_x$ according to  a uniform distribution on the interval
$[-\Delta / 2, +\Delta /2]$. The hopping parameter $t$ is set to one to
fix the energy scale and $L$ is the number of lattice sites.

In the absence of disorder ($\Delta=0$) the eigenenergies are
given by,
\begin{equation}
\epsilon_k = \frac{t}{2}\left( e^{h+ik \cdot2\pi/L} +
e^{-h-ik \cdot 2\pi/L}\right)
\label{eq:deq0spectrum}
\end{equation}
where $k = 1, 2\cdots L$.
All the eigenvalues (except $k=L/2,L$)
are complex and lie on an ellipse in the complex
plane, centered at the origin.  When disorder is turned on, $\Delta \ne
0$, the eigenvalues of the $d=1$ HNM remain confined to one dimensional
curves in the complex plane \cite{feinberg99b}, however, some of the
eigenvalues become real.  The corresponding eigenstates become localized
(Fig.~\ref{typical_V0}).
We will continue to use the notation $\epsilon_k$ for the
eigenvalues for nonzero $\Delta$ even though momentum is no longer
a good quantum number due to the breaking of translation
invariance by the disorder.  $k$ will be understood to be a generic
mode label.

\begin{figure}[h]
\includegraphics[width=0.5\textwidth]{fig1.eps}\\
\caption{(Color online) Typical spectra of the Nelson-Hatano model.
In the presence
of disorder, localized states (real eigenvalues)
appear for $\Delta$ larger than a critical value.
Half of the spectra are shown and the spectra are approximately
symmetric around the imaginary axis. The two larger up triangles
correspond to the eigenstates used for Fig.~\ref{densities}.
\label{typical_V0}}
\end{figure}

One way to understand the appearance of real eigenvalues is to consider
a system with open boundary conditions (OBC)\cite{hatano96, hatano97}.
In this case, all the eigenvalues of $\mathcal{H}_{\rm HN}$ are real,
despite the fact that the Hamiltonian is not Hermitian.  In fact, the
eigenspectrum is independent of $h$, since the $e^{\pm h}$ factors can
be ``gauged away" by a suitable redefinition $\tilde \phi(x) = e^{-hx}
\phi(x)$, of the eigenvector components.  The HNM spectrum becomes
identical to that of the Anderson model.  On a system with periodic boundary
conditions (PBC), however, this eigenvector transformation is no longer
possible, and some eigenvalues are complex (see Fig.~\ref{typical_V0}).

The dramatic difference in the spectrum between OBC and PBC
of course reflects a rather general property of the localization
transition: A localized state is insensitive to the boundary conditions
and its eigenvalue should remain real, even in the presence of PBC. On
the contrary, an extended state, for example a plane wave state, is
sensitive to the boundary conditions and its eigenvalue should be
complex in the PBC case (Fig.~\ref{typical_V0}).

Le Doussal\cite{ledoussalunp} has further clarified the relation
between the eigenvector tranformation
and the localization length by pointing out that the eigenvalues will
remain real if the localization decay $e^{-l/\xi}$ is more rapid than
the growth $e^{hl}$ induced by the transformation.  As a consequence,
the localization length $\xi$ does not
diverge at the transition, but takes on the value $\xi=1/h$
at the bifurcation point in Fig.~\ref{typical_V0} where the
line of real eigenvalues splits off into the complex plane.

For the particular case of a Cauchy distribution of
randomness, $P(\Delta)=\gamma/\pi(\gamma^2+\Delta^2)$ the location
of the bifurcation point is known \cite{hatano98} to be given by
${\rm Re} [\epsilon_k] = \sqrt{(2t\,{\rm sinh}\,h)^2 - \gamma^2}
\, /\, {\rm tanh} \, h$, and
${\rm Re}[\epsilon_k]=0$ at the critical value
$\gamma_c = 2 t {\rm sinh} h$.  At this point the randomness is
sufficiently large that all eigenvalues are real, and all
modes are localized.

More direct evidence of the localized nature of the eigenstates with
real eigenvalues can be obtained by directly looking at how the
corresponding density varies with distance\cite{hatano98}.  For example,
we can study the participation ratio $P_k$ for a given eigenvalue
$\epsilon_k$. As the Hatano-Nelson model is non-Hermitian, the left
eigenvector $\langle k | = \sum_x \langle x | \phi_{k}^L(x) $ and right
eigenvector $|k\rangle  = \sum_x \phi_{k}^R(x) |x\rangle$ are not
Hermitian conjugates.  It was shown\cite{hatano98} that the probability
density in these systems is given by $\left|\phi_{k}^L(x)
\phi_{k}^R(x)\right|$ which is a better behaved quantity
than $|\phi_{k}^L(x)|^2$ or $|\phi_{k}^R(x)|^2$
although they give quite similar results for localized states (Fig.~\ref{densities}).

\begin{figure}[h]
\includegraphics[width=0.5\textwidth]{fig2.eps}\\
\caption{(Color online) Three different possible definitions of the density in an
extended (left) and localized (right) states corresponding to
different eigenvalues $\epsilon_k$ of the same system. In general
$|\phi_{k}^{L,R}(x)|^2$
show quite strong fluctuations, thus making $\left|\phi_{k}^L(x)
\phi_{k}^R(x)\right|$ a better quantity to identify the different states.  \label{densities}}
\end{figure}

Then the participation ratio $P_k$ can be
defined as,
\begin{equation}
P_k = \frac{1}{L}\sum_x \left|\phi_{k}^L(x) \phi_{k}^R(x)\right|^2
\label{eq:participation}
\end{equation}
$P_k$ corresponds to the portion of the lattice sites that is occupied
for a given eigenvalue. It goes to zero for a localized state
in a large system and goes to a number of
order unity for an extended state when
the density distribution is spread
equally over all the sites.
Fig.~\ref{quantities}
shows that the vanishing of the participation ratio aligns
nicely with the energy
at which the eigenvalues are real. Similar participation ratios can be
defined with other definitions of the density $P^{L,R}_{k} = \sum_x
|\phi_{k}^{L,R}(x)|^2/L$. But, as for the densities
(Fig.~\ref{densities}) themselves, $P_k$ is better behaved than
$P^{L,R}_k$.

The current $J_k$ defined as $J_k = -i \partial \epsilon_k / \partial h$ \cite{hatano97} is
compared with the participation ratio in Fig.~\ref{quantities}. It gives similar
results for the extended or localized nature of the states, but is more difficult to calculate as it requires a numerical
derivative (and then two diagonalization instead of one for the participation ratios) and
is difficult to define close to the mobility edges.

\begin{figure}[h]
\includegraphics[width=0.5\textwidth]{fig3.eps}\\
\caption{(Color online) Different quantities which distinguish the extended from the localised
states in the Hatano Nelson model: the imaginary part of the eigenvalues
${\rm Im}(\epsilon_k)$, participation ratio $P_k$,
and real ${\rm Re}(J_k)$ and imaginary ${\rm Im}(J_k)$ parts of the current.
All these quantities give consistent information
concerning which modes are localized or not.\label{quantities}}
\end{figure}

\begin{figure}[h]
\includegraphics[width=0.5\textwidth]{fig4.eps}\\
\caption{(Color online) With the periodic potential, a gap is opened for
$V > V^{\rm o}_{\rm c} = t \sinh(h)$ although all the states remain extended.
$V^{\rm o}_{\rm c} \simeq 0.636$ in the case shown, $t=1.0, h=0.6$.\label{typical_D0}}
\end{figure}

\subsection{Effect of a periodic potential}

Our interest here is in adding
a simple potential of period 2 to the original HNM,
\begin{equation}
\mathcal{H} = \mathcal{H}_{\rm HN} + \sum_{x=1}^L V \cos(\pi x)  n_x
\end{equation}
When $h=\Delta=0$, this term
generates a spectrum with two bands separated by a gap of
width $2V$.
In the non disordered case where
$h \ne 0$ and $\Delta = 0$ we obtain the following eigenvalues
\begin{equation}
\epsilon_k = \pm \frac{t}{2}\sqrt{4V^2/t^2 + 2 + e^{2h+ i k \cdot 2 \pi/L}
+ e^{-2h -i k \cdot 2 \pi/L}}
\end{equation}
with $k = 1, 2\cdots L/2$. In this ordered case, the spectrum has a gap if
$V > V^{\rm o}_{\rm c} = t \sinh(h)$ and its width $W_{\rm G}$
is given by
\begin{equation}
W_{\rm G} = 2\sqrt{V^2 - t^2 \sinh^2(h)}
\end{equation}
Even when $\Delta = 0$, there is a transition
in this model corresponding to the opening of the gap at
half-filling (see Fig.~\ref{typical_D0}).
The gap opens with exponent
$\beta=1/2$ since near
the transition
$W_{\rm G} \simeq \sqrt{2V^{\rm o}_{\rm c}(V-V^{\rm o}_{\rm c})}$.

\section{Phase diagram}

In the presence of both disorder and the periodic potential,
the spectrum of the model can show several different topologies.
We calculate the eigenspectrum for one disorder realisation of a large size system ($L=1000$)
and analyse
the different topologies appearing.
We checked that these topologies were still
present for other sizes ($L=500, L=2000$) and other disorder realisations.

Scanning horizontally along the real axis in the complex eigenvalue
plane, we observe three types of regions in the spectrum. First we
observe cases of real eigenvalues corresponding to localized (L)
states. Second we observe regions with complex eigenvalues corresponding
to extended (E) states. Finally we observe some gaps (G) in the
spectrum. A given topology is characterized by the succession of these
different regions as one increases the real part of the eigenvalue, ${\rm
Re}(\epsilon_k)$.  The different topologies we observed are shown in
Fig.~\ref{difftypes} and their position in the $(V,\Delta)$ plane for a
fixed value $h=0.6$ is shown in Fig.~\ref{phasediagram}.  As an example,
the phase shown in Fig.~\ref{difftypes}(a) is denoted as the LEL phase
since we observe a central region of extended states (E) between
two regions of localized states (L) with no gaps.

\begin{figure}
\includegraphics[width=0.5\textwidth]{fig5.eps}
\caption{(Color online) Different topologies of the eigenspectrum
for one realization of a $L=1000$ system and for $h=0.6$.
The simple E topology (only extended states without a gap) and
the rarely observed LELEL are not shown.
See text for discussion.
\label{difftypes}}
\end{figure}

\begin{figure}
\includegraphics[width=0.5\textwidth]{fig6.eps}
\caption{(Color online) The different phases observed in the Hatano-Nelson model for a given realization
on a $L=1000$ system size and for $t=1, h=0.6$. At the boundary
between different phases, the behavior is sometimes irregular
for a finite size system
and does not fall into one of the identified categories. The labels (a)-(f)
correspond to the cases shown in Fig. \ref{difftypes}.
\label{phasediagram}}
\end{figure}

The location of these different phases  for $h=0.6$ is shown in Fig.~\ref{phasediagram}
for a given realization.
As expected, a gap appears for $V$ large enough. For moderate disorder
($\Delta < 2$), the opening of the gap happens approximately at the same
value $V^{\rm o}_{\rm c}={\rm sinh}\,0.6=0.636$
as in the ordered, $\Delta=0$ case.  Upon increasing
$\Delta$, the original low disorder E and EGE phases are modified as
some of the extended states are transformed into localized ones at the
edges of the extended regions, leading to the LEL and LELGLEL (or LEGEL)
phases respectively. In the LEGEL phase, localization first appears on
the external edge of the extended regions and not on the border of the
gap.  This is consistent with the fact that localized states
appear first for the extremal eigenvalues in the Anderson model.

In a very small region of the phase space, we also observe a LELEL
phase where the region between the
two extended blobs is filled by localized states but no gap
appears.  As $\Delta$ is
increased further, all the extended states disappear leading to the
large disorder L and LGL phases.  When $V$ and $\Delta$ are both large,
the transition from the L phase to  the LGL  phase occurs at $V_{\rm c}
= \Delta/2 $ which is the result expected in the one site limit, when
the hopping terms are neglected. In the one site limit the gap opens
like $W_{\rm G} \simeq 2(V-V_{\rm c})$ which is a different behavior
from the opening of the gap due to the periodic potential.

For a given realisation, close to the boundary
between two phases, the spectrum becomes disordered
and it is difficult to classify it as
belonging to one of the simple topologies identified before.
These regions are indicated by ``$\times$"
in the chosen example (Fig.~\ref{phasediagram}). To calculate
more precisely the boundaries between the different phases,
it is then necessary to use different quantitative indicators
and to average those over several disorder realisations.
First we measure the width of the gap
in the system and determine whether it is present or  not.
Second we determine if the spectrum is made of
complex values (extended states) only, of a mixture of complex and real values
(extended and localized states), or of real values only.
We consider a $L=1000$ system and average over 10 realisations.
Drawing these three lines in the phase space, we obtain the
phase diagram shown in Fig.~\ref{phasediagram2}. With these
quantities, we cannot distinguish the LELGLEL from the
LEGEL phases, as well as the LELEL from the LEL phase.

\begin{figure}
\includegraphics[width=0.5\textwidth]{fig7.eps}
\caption{(Color online) The phase diagram obtained by averaging several disorder realisations
to calculate
the boundary between different regions.  The smooth lines are fits to the data.
The continuous green line marks the limit between gapped
and ungapped regions. The dotted blue, the limit between a spectrum without any
real values and a spectrum with real and complex values. The dashed red line is the limit
between a spectrum with real and complex eigenvalues and a spectrum
with only real values.  \label{phasediagram2}}
\end{figure}

We observe an interesting reentrant behavior. If the system is in the
EGE phase but the gap is not too large, when we increase $\Delta$,
the gap will be closed by the disorder but the states in the middle
of the spectrum will remain extended (Fig.~\ref{reentrant}).  Then we observe a
transition where increasing disorder drives the gapped system
into an ungapped phase. This can be understood as follows: as the disorder
is increased, the E regions have a tendency to flatten out as
they evolves towards L regions with only real values. By doing so,
the E regions spread along the real axis. If the gap is not
to large, two gapped E regions can then merge in the process, which
is happening here.
\begin{figure}
\includegraphics[width=0.5\textwidth]{fig8.eps}
\caption{(Color online) For $V=0.7$, upon increasing the disorder, the gap $W_G$ is closed
before the states becomes localised, which is shown by the participation ratio $P$ becoming zero.
Here, the quantities are averaged over only 5\% of the total
number of eigenstates located in the middle of the spectrum,
to get rid of possible bias induced by states located at the edges
of the spectrum.  The measurements show the crossings of the two boundaries
of the phase diagram at largest $\Delta$ (gap closing and
all extended states vanishing) for $V=0.7$ in
Fig.~\ref{phasediagram2}, but not the crossing of the boundary at
smallest $\Delta$ when localized states first appear.
\label{reentrant}}
\end{figure}

\section{Transitions}

\subsection{Opening of the gap}

As expected, we observe two different behaviors for the opening of the
gap for a fixed value of $\Delta$ as $V$ is increased (see Fig.~\ref{gapopening}).
If $\delta = V-V_{\rm c}$, we
have a behavior $W_{\rm G} \propto \sqrt{\delta}$ as in
the non interacting regime, whereas
$W_{\rm G} \propto \delta$ in the strongly disordered regime
Fig.~\ref{gapopening}. The transition between those two different behaviors
happens precisely at the point where, in the phase diagram Fig.~\ref{phasediagram2},
we are passing from the low disorder into the large disorder regime.
For $\Delta < 2$, the transition almost takes place at the non-interacting
critical value $V_{\rm c}^{\rm o}$, the transition occurring at nearly constant
$V$ and with the square root behavior.
Above this value, the transition takes place approximately
at $V_{\rm c} = \Delta /2$ with the linear behavior,
which is characteristic of the disordered regime.
\begin{figure}
\includegraphics[width=0.5\textwidth]{fig9.eps}
\caption{(Color online) Evolution of the gap as a function of $V$. For $V< 2.0$, the gap
opens like $W_{\rm G} \propto \sqrt{V-V_{\rm c}}$
as in the non disordered case. For $V \ge 2.0$, the
opening of the gap is linear as expected for a transition in the disorder regime.
\label{gapopening}}
\end{figure}

\subsection{Finite size analysis of the localization transition}
\begin{figure}
\includegraphics[width=0.5\textwidth]{fig10.eps}
\caption{(Color online) Finite size scaling analysis of the participation ratio.
For this value of $V$, the transition towards localization happens
at $\Delta_{\rm c} \simeq 2.5$.\label{scaling}}
\end{figure}

It is possible to analyze more precisely the transition to the localized
regime by performing a finite size analysis of the participation ratio.
We define the mean participation ratio $P = \sum_k P_k / L$ which becomes
zero when we have only localized states.
We found that the participation ratio is varying linearly with the size
of the system $L$. In Fig. \ref{scaling} we show the result of a finite
size analysis for a given value of $V$ and for different values of
$\Delta$. We see that $P$ extrapolates to zero for values larger
than $\Delta_c \simeq 2.5$. This is in agreement with the phase diagram
obtained with a $L=1000$ size (Fig. \ref{phasediagram2}).

\section{Conclusion}

We have studied the Hatano-Nelson model in the presence of a periodic
potential.  We have determined the phase diagram of the system and shown
that it presents a variety of different localized or gapped phases,
distinguished by the topology of the eigenspectrum in the complex plane.
Interesting insulator-metal transitions can occur, driven by increasing
disorder. Finally, we have determined how the gap and participation
ratio evolve close to these transitions.

There are some interesting analogies between eigenspectra
features induced by a periodic potential, discussed here,
and those which appear in crossing over from one
to two dimensions \cite{zee98}.
We comment first that the $d=2$ model can be trivially
solved in the clean limit $\Delta=0$ with hoppings
$t_x, t_y$ and non-Hermiticity parameters $h_x,h_y$.
In fact, the eigenvalue distribution in the
complex plane is obtained by taking
ellipses determined by $t_y$ and $h_y$, and placing them with
centers at each
of the eigenvalues of Eq.~\ref{eq:deq0spectrum}.  In the limit
of large lattice sizes these eigenvalues become space filling in
the complex plane.

However, just as discussed here, different topologies are possible.
If $t_y$ and $h_y$ are small compared to $t_x$ and $h_x$ (or
{\it vice-versa}) one is overlaying small ellipses on a background of
a larger ellipse, and the eigenspectrum retains a hole in the origin.
When the hoppings in the two dimensions are comparable,
in contrast, the central hole can get filled in.
It is not surprising that a particularly close analogy
is obtained by considering a system consisting of two chains since
such a situation describes, as with the periodic potential
considered here, a lattice with two different types of sites (two bands).
The resulting eigenvalue spectra reflect considerable similarities
with those found in this paper.
See, for example, Fig.~2 of [\onlinecite{zee98}].

Random non-Hermitian matrices also arise in the study of quenched
Quantum Chromo-Dynamics at finite quark
density.\cite{stephanov96,halasz97}  While the structure of the
matrices does not take the precise form of the HNM, it is
interesting that in certain cases (``Dyson index" $\beta=4$) a gap
appears in the spectrum in the complex plane, analogous to that found
here.\cite{halasz97}
That is, the eigenvalue distribution can be driven to zero in
a region in the vicinity of the imaginary axis, not unlike the
effect of increasing $V$ in Fig.~\ref{typical_D0}.  (In these studies the
spatial dimensionality is greater than one so that the eigenvalues
are space filling as opposed to lying along one-dimensional curves.)
Indeed, a key result\cite{stephanov96} is that
the appearance of a gap around the imaginary axis
requires a finite value of the appropriate tuning
parameter, the chemical potential $\mu$, much as our phase diagram
(Fig.~\ref{phasediagram}) requires a finite staggered
potential $V > V_c \simeq 0.7$ for
the appearance of a gap.

The original motivation for the HNM was the problem of flux line
motion in type II superconductors.
Specifically, deliberate heavy ion irradiation
\cite{CivaleReview} produces
random tracks along which the flux lines like to sit, and
a transverse magnetic field then provides the 'non-Hermiticity'
which attempts to delocalize them.  It is also possible to
provide regularly patterned pinning centers, which would be a
realization of the staggered $\pm V$ term in the extension of the
HNM presented here.\cite{baert95,harada96,reichhardt96}
Our phase diagram,
Fig.~\ref{phasediagram} indicates that the amount of random
disorder $\Delta$ required to produce localized phases in
general increases with the amplitude $V$ of the patterned
potential, so that critical currents would decrease
as patterned pinning centers are established if the modulation
is at the atomic level.  It would be interesting to study the
effect of regular variation in the site energy at longer length
scales, such as would more typically be accessed in experiments
with patterned pinning.

\begin{acknowledgments}
We acknowledge support from the National Science Foundation under
award NSF-ITR-013390, the  Natural Science Foundation of Shanghai (10ZR1403400), and
ARO Award W911NF0710576 with
funds from the DARPA OLE Program.
This work was also supported by the CNRS-UC Davis EPOCAL LIA joint research grant. The authors
would like to thank B.~Holly and B.~Gr\'emaud for useful input. Z. Bai and R.T.~Scalettar
wish to thank the hospitality of Fudan University where portions
of this work were done.
\end{acknowledgments}


Benny and Franz are thieves. The brother steal jeans in shopping centers and boutique stores. Their routine involves a scam in which Benny, the younger of the two, has to play the ungrateful role of the decoy. When they encounter an overstrung shop assistant, it becomes clear to Franz that Benny's not going to let himself be pushed around very much longer.


Special Director's desk to view all reports on a single screen. No more navigation and site maps to be remembered to view reports. Online Audit allows you to freeze the data once it is checked and verified. It is authentic and reliable data that matters and not just data which is relevant.


text:
Top 10 under 40: Asaf Levy, Metro Supply Chain Group
By CS Staff May 15, 2020
News Top 10 Under 40 Metro Supply Chain Group top 10 under 40
Clothing, car parts and cannabis. These are just three of the commodities that Asaf Levy might have eyes on in a typical day in his role at Metro Supply Chain Group, a logistics firm that manages storage and last mile delivery of a spectrum of goods for a wide variety of clients.
Levy says his company manages 12 million square feet of storage across the country, as well as other locations in the U.S. and U.K. His role involves writing standard operating procedures (SOPs) and overseeing standards compliance and security systems design. Lately, cannabis, and all the issues that come with that, has taken up many of his working hours.
"That's been my main focus this year, just because the industry is so brand new," he explains.
"The nice thing is, the company is always working with new clients, so every new client has their own security," he adds. "So I kind of liaise with their security and make sure our SOPs and standards mesh well, especially in the cannabis world. There's a lot of regulations that we need to meet, so liaising with their head of security and making sure that they're happy is really what it comes down to."
Levy also sits on ULC's cannabis standards council and interacts with Health Canada as the relatively new legal recreational cannabis industry finds its footing.
Levy says his client interactions range from relationships with senior security managers to mom and pop retailers — in the latter case he may become their de facto security consultant.
"Sometimes it's walking them through processes and getting them to understand," he says.
Levy got his start in loss prevention as a mall security guard, then site supervisor. His initial goal was a career in law enforcement but he became more engaged with security as a plain clothes loss prevention operative for The Bay. He worked at several other retailers, including Amazon, before finding his role with his current employer.
His latest passion is cybersecurity and he is currently enrolled in a cyber program at Toronto's York University.
"Learning about how to lock down IT infrastructures from a security perspective has become my new goal. I feel like a lot of things are going that way."
TrackTik Software CEO receives technology innovation award
Top 10 under 40: Terri Govang, WSP Canada Group Ltd.
Top 10 under 40: Robert Hastings, Manulife
Top 10 under 40: Adam Hutchings, Canada Energy Regulator
Top 10 under 40: Richard Leborgne, Montfort Hospital Ottawa
Top 10 under 40: Brine Hamilton, GardaWorld


The more mobile a person with dementia remains, the better it will be for their health, and the easier for those around them to manage.
The more mobile the person remains, the better it will be for their health, and the easier for those around them to manage. Look for ways to help the person remain mobile.
If the person becomes unsteady on their feet, an occupational therapist should be able to provide information on aids and equipment, such as grab rails, to help them move around.
If the person spends a lot of time sitting down, they will need a firm, comfortable chair that is easy for them to sit down in and get up from.
If the person needs support when they move around, an occupational therapist or physiotherapist can give advice on how carers can safely give them the support they need without injuring themselves.
There are many chair based exercises that can help someone to stay mobile, such as raising legs in isolation.
Exercise is beneficial to everyone, whether or not they have dementia, and everyone who is capable should get some exercise. There are lots of different types of exercise that can be adapted to individual preferences and abilities. For example, there are lots of seated exercises for people who have difficulty walking. Try to find a form of exercise that will be enjoyable - ask the GP, occupational therapist or physiotherapist for suggestions.
reduce anxiety, stress and depression.


Using the Leadbelcher base spray made painting a lot quicker as a very large bart of this model is just Ironbreaker layered over Leadbelcher with Nuln Oil shade and Runefang Steel edge highlight. I tried using the Mephiston Red spray on the non-metallic shell, but I found the colour came out a lot darker than the potted paint and I had to coat over it a few times anyway.
The stripes were somewhat intimidating to do. I started out trying to use masking tape to divide the sections bit this ended up being messier than freehanding it with a long lining brush. The large white section in the middle that denotes the princeps rank was a little daunting as I have always had trouble with the White Scar paint. In the end I painted it Ulthuan Grey then layered/highlighted it with White Scar.
I think some of the transfers are slightly rotated and off centre, but it is not too noticeable unless you are looking for it. There is some Blood for the Blood God technical paint splattered over the chain sword which I applied by flicking it from a thick brush, and I really like the effect it gives.
The base was done with crackle paint layered over red and orange streaked base and topped with black paint. If there are any ideas for extra bits of scatter to make it look more interesting, I would love to know as I am coming up blank.
Overall, I am very happy with how this model turned out and I am looking forward to painting the Knight Princeps model when my preorder arrives next week. Thank you for reading!
That looks great! Impressive amount of magnetization work, too.
Mephiston red spray, I think might be a closer match for Khorne red, but I'm not sure. The GW sprays are too expensive for my taste, so I don't have any experience with them.
Cavalier over at Frontline Gaming turned me on to a good trick for white: Start with Celestra grey, then cover all of that except the crevices and such with Ulthuan grey. You don't even need to go to White Scar/Ceramite white in most cases, because the Celestra grey makes for enough contrasting shading that the eye registers the Ulthuan grey as white.
The base looks fantastic. I wish I could manage to get crackle paint to work that well for me. As far as little bits to mix it up a bit, what I would do is break up more cork into really tiny pieces, small enough that there's only one flat side, which gets glued to the base, or to a flat layer of cork. It also helps if you have a couple of different sizes of cork available to mix it up more, and make it less obviously sheets of cork. I might also give the rocks some very light highlights in a dark red/orange. Just enough to give them some definition, not so much that it's really consciously noticeable.
Even without that, tho, that is excellent work, and I look forward to seeing the whole lot of them together!
I will try that white trick! It is very interesting how our eyes process things relating to colour.
The varying sizes of cork sounds like an excellent idea, I will have a look through my materials shelf and see if I have some different sizes of cork. Thank you very much!
This looks great I have 3 knights to build and 2 to paint myself (converting one for a friend for Christmas). Seeing really nice work like this is a great motivator. Really lovely stuff.


HELENA, Mont. -- Democratic and Republican state political party committees raised $1 billion of soft money over a four-year period covering the 2000 and 2002 election cycles, with Florida leading all states by a wide margin, a new, 50-state study shows.
In Florida -- where the 2000 presidential race erupted in controversy and 2002 held a gubernatorial re-election contest featuring President Bush's brother -- the two main state committees raised $153 million over four years. They far outpaced California party committees, which ranked second at $79.4 million, the study by the Institute on Money in State Politics showed.
Slightly less than half of the money came from the six national party committees, which can no longer raise the soft money they gave their state counterparts in such abundance.
"Last week's U.S. Supreme Court ruling leaves big-money donors looking for new places to give their soft money and state party committees looking for ways to replace the millions of dollars they received from the national parties," noted Edwin Bender, executive director of the Institute. "It's quite likely these two groups will meet up in the future, and many donors will be funneling their money directly to the states -- where it will be harder to track through 50 different sets of laws and state disclosure agencies."
The Institute is a national nonpartisan, nonprofit organization that collects and analyzes campaign contribution reports for state-level candidates and party committees. Its database of information is available on the Web at www.followthemoney.org.
"Our study of past giving to party committees will provide a baseline for measuring how changes in federal campaign-finance laws will affect giving to state party committees in the future," Bender said.
The Bipartisan Campaign Finance Reform Act, upheld last week by the U.S. Supreme Court, banned soft-money contributions to national party committees and placed other restrictions on the use of soft money.
The Institute's study, supported by a grant from The Pew Charitable Trusts, found that national political party committees contributed 44 percent of the soft money that went to state party committees in the 2000 and 2002 election cycles -- $255 million in 2000 and $217 million in 2002.
"Already, those committees have lost $46 million in funds they had received from the national committees by this same point in the 2000 presidential cycle, a cycle comparable to the current election cycle," Bender noted. "What remains to be seen is whether this money now flows to the state party committees through other sources or whether it simply disappears from the political system. But past experience tells us that political money usually finds its way around obstacles."
Should money once contributed at the national level find its way to the state party committees, tracking the funds will become more difficult, Bender said, explaining that 50 different state laws and state agencies would be regulating contributions that once were governed by one federal law and reported to one federal agency.
-- The five top-contributing industries remained the same in each election cycle: lawyers and lobbyists, real estate interests, public sector unions, general trade unions, and securities and investment interests. Giving by these five industries totaled $128.2 million during the study period.
-- Contributions from individuals represented only 14 percent of the total giving in 2000 and 16 percent in 2002. But the top 25 individual contributors in each of the election cycles gave 15 percent of the $160.7 million given by individuals.
-- Three individuals gave more than $1 million to state party committees in the 2000 election cycle: Silicon Valley executive Steven Kirsch of California, S. Daniel Abraham of Slim Fast Foods in Florida, and computer hardware developer Bernard Daines of Washington state. Kirsch gave $2.15 million to Democratic committees in 10 states, Abraham gave $1.3 million to Democratic committees in 19 states, and Daines gave nearly $1.2 million to Republican committees in five states.
-- Only one contributor gave more than $1 million in 2002: James Pederson, a real-estate developer and chairman of the Arizona Democratic Party. He gave $3.7 million, with all but $1,000 going to the Arizona Democratic Party.
-- State party committees also sent money to committees in other states, sometimes in exchange for hard money that could be spent directly on federal election activities and candidates. The state committees gave more than $6 million to their counterparts elsewhere over the study period.


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The Herman Cain Story: Is the Liberal Media Dead? »« Republican Establishment Smears Herman Cain . . . and the Tea Party
Phony Herman Cain Smears from a Band of Gold-Digging, Democrat Bimbos
As the democrat bimbos are considering joining forces to see whether they can assemble enough gold-digging, floozy operatives to create one credible-looking sexual harassment accusation, we are finding out more about the two women who have come forward so far.
Sharon Bialek, also known as the fourth accuser, is a woman with an unsteady string of jobs, chronic bankruptcy, and a failed paternity suit against a different executive. Along with being represented by the liberal, democrat Gloria Allred, Bialek has been conveniently located in the same apartment building with President Barack Obama's senior advisor David Axelrod.
Oh, by the way, Sharon Bialek and her recently unemployed fiance, Mark Harwood, are both unemployed and would probably like the money that high-profile television appearances might bring – to say nothing of the payoffs they might be receiving as well. How do two unemployed people afford a high-end apartment and a high-priced lawyer like Gloria Allred. Those unemployment checks in Illinois must be really big.
Then there's the original Cain accuser, who would not come forward before, Karen Kraushaar. We have some idea why now. It seems Kraushaar, who was so eager to speak until the NRA was agreed to release her from her agreement, made a complaint against her next employer, just after her complaint against Herman Cain at the National Restaurant Association.
Among other things, that complaint accused a manager of circulating a sexually charged email. According to the AP, Kraushaar "considered her employment complaint 'relatively minor' and she later dropped it." In other words, even Karen Kraushaar now admits that she made a frivolous complaint.
bialek, bimbo, democrat, herman cain, Karen Kraushaar, Mark Harwood, sexual harassment, sharon