Commercial leases are contracts used to rent property to another person so that the person can run a business on the premises. Every business is different and each piece of real-estate is unique. There is no such thing as a "one size fits all" commercial lease. Like everything else in business, the terms of a commercial lease are subject to negotiation.
Will the Tenant pay a fixed base rent, a percentage of gross sales, or both?
Does are the rent increases and how much are they?
How long is the first term of the lease?
How long are the option terms?
Does the lease automatically renew?
Does the tenant pay to keep up the landscaping?
Is there a threshold for minor repairs?
Is there a cap for major repairs?
Is the tenant required to pay sales tax as a part of the rent?
Who pays what types of insurance and how much coverage?
Is there an early termination clause?
What happens in the event that the Landlord sells the building?
There are many differences between residential and commercial leases. For example, in a Commercial Lease you often have terms of 10 years or more. When you add options and renewals to the lease, you may have a contract that will last longer than you will be alive. The longer the lease, the greater the chance that there will be a problem. Whether you are the Landlord or Tenant, you need to understand the lease and take steps to prevent minor issues from becoming problems.
Without an understanding of the issues that are likely to arise during and at the end of your lease, you will not know what you should put in your lease. If you are have commercial property or are looking to rent then make a list of the issues related to the business and the property. Use that list to guide you in drafting your commercial lease. After you finish the list then you may want to contact a lawyer to check the issues and give suggestions.


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SECTION 1 - SCOPE OF APPLICABILITY
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redpajama_set_name: RedPajamaCommonCrawl


"The Chicago Youth Boxing Club provides professional boxing instruction to youth in Little Village, North Lawndale, Humboldt Park and some suburbs. Victor Rodriguez, Gabriel Navarro and Ana Patricia Juarez discuss their work and growth of the organization."
"CYBC provides a positive and healthy environment for Chicago's inner city youth; instilling positive and productive skills, and discipline, through boxing and team environment," the organization's Facebook page says.
"Established in 2001, The Chicago Youth Boxing Club was originally established to promote youth boxing and raise funds to support youth entrance fees into local and national competitions. Since 2001, CYBC has evolved into a non-profit organization dedicated to the social, educational and physical well being of Chicago's inner-city youth. Working with its community partners Little Village Community Development Corporation and the La Villita Community Church.
"CYBC opened its permanent home in Little Village in the Fall of 2007. This facility serves not only as a community gym, but also as a home to the CYBC youth program. In this time, CYBC has grown to include several volunteer, part-time staff, and a full time coach as well as program management staff who serve 35-40 youths daily."
"Just like boxing saved me, I'm trying to save others"
"It's a boxing club, obviously, but it's more youth development than anything else."


text:
Santa Llúcia de Casa Aytés és la capella particular de Casa Aités, en el poble d'Enviny, del terme municipal de Sort, a la comarca del Pallars Sobirà. Pertanyia a l'antic terme d'Enviny. Està situada a Casa Aytés, dins del poble d'Enviny, a la seva zona central-oriental. Actualment (principis del segle XXI) és en ruïnes. És una obra inclosa a l'Inventari del Patrimoni Arquitectònic de Catalunya.

Senzilla construcció de planta rectangular amb capçalera a ponent i porta a l'est, per damunt de la qual s'obre una petita roassa. La façana es troba coronada per una espadanya d'un sol arc i els murs laterals presenten contraforts a l'exterior. Actualment la coberta es troba ensorrada.

Referències

Bibliografia

Enllaços externs
 Santa Llúcia de Casa Aytés en el seu entorn, a l'Institut Cartogràfic de Catalunya

Esglésies de l'antic municipi d'Enviny
Patrimoni monumental de Sort

redpajama_set_name: RedPajamaWikipedia


text:
La Ferrari 296 GT3 est une voiture de Grand tourisme développée par Ferrari et assemblée par Oreca répondant à la réglementation technique GT3.

Aspects techniques
La Ferrari 296 GT3 est une voiture de Grand tourisme répondant à la réglementation technique GT3. Celle-ci est donc éligible à de nombreuses compétitions automobiles telles que celles organisées par l'ACO, l'IMSA ou le SRO.

Elle est basée que la Ferrari 296 GTB et a été entièrement conçue à Maranello par une équipe dirigée par Ferdinando Cannizzo, responsable de la conception et du développement des voitures de course GT. Elle sera assemblée dans les installations d'Oreca à Signes à partir de 2022. Contrairement à la Ferrari 296 GTB, elle n'est pas équipé de système hybride rechargeable afin de répondre à la réglementation en vigueur. Oreca assurera également le support client. Les premiers tours de roues sont prévus pour le premier semestre 2022.

Le , Ferrari a publié les premiers visuels de sa 296 GT3.

Dans une logique de rendre sa voiture accessible à tous les pilotes et notamment aux amateurs, Ferrari a travaillé sur l'équilibre de la 296 GT3. L'équilibre aérodynamique et les mouvements de caisse ont été réduits de 20% à l'avant et de 40% à l'arrière par rapport à la 488 GT3 selon Stefano Carmassi, responsable développement piste des GT chez Ferrari,

Histoire en compétition

Notes et références

Lien externe

296 GT3
Voiture de course
Automobile des années 2020


St Mary and St Margaret Church is unusual and unique in that it is a church within a church - a Norman and medieval church within a Georgian one.
It is believed worship has happened at the site for over 2,000 years. The earliest known building was a small wooden Norman chapel on the site before 1175. The chapel was remade of stone in the 12th century and in the 15th century the Norman chapel had a large half timbered structure and wooden tower added to the west end.
Castle Bromwich Hall was rebuilt in the 1700's using local clay bricks and the old timber church was encased in brick and plaster. The massive oak roof trusses can now only be seen in the attic above the plaster ceiling.
The original Church hall was small, had limited facilities and could only be used by a small group at a time which no longer met the needs of the growing community. In 2009 Castle Bromwich PCC secured planning permission to build a new community hall next to the existing Grade 1 listed Church.
Castle Bromwich PCC applied to Biffa Award for funding through the Landfill Communities Fund to build the proposed hall with the aim of enabling local residents and organisations to provide a wider range of services to the community. The newly built hall includes kitchen facilities, an accessible meeting room, an office space and accesible WC's inlcuding baby change facilities.
The hall took 17 years to complete with a total cost of £435,000. The work was funded through a mix of donations, a loan from the local diocese, fundraising and the LCF. Through Biffa Award, £50,000 was contributed from the LCF.
The hall is now widely used by the community for a range of activities including yoga classes, a community run playgroup, an exercise class for the over 50's, a luncheon club for the elderly of the parish, a bereavement support group as well as a weekly drop in centre for the whole community which provides a place to meet, chat and relax while taking advantage of the tea, coffee and biscuits that are served for a small donation.
The building is open to the public throughout the year Monday to Friday from 8am to 10pm, 9am to 10pm on Saturdays and from 12.30pm to 6pm on Sundays. Access to the building is free of charge for some activities and the booking process can be accessed through the church website. The hall can also be rented at competitive rates for parties, private events and corporate hire with in-house catering options available.
Through additional fundraising activities the Church has also now landscaped the gardens around the hall providing a quiet, reflective space for people from across the community to come into and enjoy. They have also developed a paved walkway where bricks can be purchased in different areas and messages are carved onto the bricks for celebrations, in memoriam and to give thanks.
Background and history courtesy of William Dargue & David Adams 2004, A Brief History of Castle Bromwich and its Church.


text:
\section{Introduction}\label{sec:intro}

In ordered magnetic insulators, spin waves can transport spin and heat without an actual motion of electrons~\cite{Akhiezer1968,Kajiwara2010,Kruglyak2010,Bauer2012,Uchida2010,Chumak2015,Nakata2017a}. The corresponding bosonic quasiparticles - magnons - bear several properties distinct from electrons~\cite{Demokritov2006,Takei2014,Sonin2010,Flebus2016,Bozhko2016,Bozhko2019,Brataas2020,Yuan2018,Sonin2020,Kamra2016,Kamra2017}, which make them interesting from both physics and technological perspectives. Due to the generally non-conserved nature of spin, a range of phenomena not admitted by electric current become feasible. Exploiting this principle, coherent spin waves generated using a microwave antenna can be amplified via various mechanisms, such as charge current~\cite{Akhiezer1968,Akhiezer1963,Spector1968}, spin transfer torque~\cite{Seo2009,An2014,Graczyk2021,Padron-Hernandez2011}, and thermal gradient~\cite{Padron-Hernandez2011a,Brechet2013,Yu2017}. Furthermore, attributes such as chirality can be bestowed upon the different spin wave modes via engineering of the energy landscape in the host magnet~\cite{Nembach2015,Gladii2016,Kim2016,An2013,Mook2016,Moon2013,Cortes-Ortuno2013,Garst2017,Tokura2018,Yu2021,Wang2020}.

Spin transport via incoherent magnons, i.e., by a drive such as temperature that does not select a single mode, has also been proposed and demonstrated~\cite{Uchida2010,Cornelissen2015,Bauer2012,Brataas2020}. As a prominent example, nonequilibrium magnons and spin can be injected electrically into a magnetic insulator using a heavy metal electrode~\cite{Zhang2012,Zhang2012a,Cornelissen2015,Goennenwein2015,Li2016,Cornelissen2016,Sinova2015,Velez2016}, made from platinum, for example. Detecting these by a spatially separated electrode provides crucial insights into the nature of spin propagation in the magnet~\cite{Han2020,Takei2014,Zhang2012}. Such a nonlocal method has been inspired, in large part, by the corresponding studies of electronic spin injection and detection in metallic and semiconducting systems~\cite{Johnson1985,Takahashi2003,Fabian2007,Zutic2004}. In the latter, spin chemical potential characterizes spin transport. In a similar fashion, magnon chemical potential~\cite{Cornelissen2016,Bender2012} has been found to play the dominant role in nonlocal spin transport studies employing magnetic insulators.

Taking further inspiration from this similarity, one may consider the possibility of modulating the magnonic spin propagation length in nonlocal transport studies using pre-existing drift currents. Such effects have previously been demonstrated for electronic spin transport~\cite{Fabian2007,Appelbaum2007,Huang2007,Kameno2014,Ingla-Aynes2016}, and has recently been observed in the context of magnonic spin transport~\cite{Schlitz2021}. Once again, unique properties of these non-conserved magnons should enable novel drift mechanisms associated with, for example, the chirality of eigenmodes~\cite{Nembach2015,An2013,Wang2020,Schlitz2021,Yu2021}.

In this article, inspired by the similarity between nonlocal spin transport in electronic and magnonic systems, we theoretically examine the emergence of drift currents and concomitant control of spin propagation length in magnonic systems. We first establish the drift phenomenology for magnons thereby clarifying its qualitative role in nonlocal magnon transport experiments. Equipped with these insights and using the Boltzmann equation approach~\cite{Kittel2004,Chen2005,Cornelissen2016}, we examine three representative mechanisms that may cause magnon drift - magnetic field gradient~\cite{Meier2003,Kosevich2013,Liao2014,Basso2016,Mook2016,Mook2018,Nakata2015,Nakata2017a}, asymmetric contribution to dispersion~\cite{Gladii2016,An2013,Mook2016,Moon2013,Cortes-Ortuno2013,Schlitz2021,Yu2021,Mook2014,Kim2016,Kim2016a}, and temperature gradient~\cite{Sanders1977,Xiao2010,Adachi2011,Uchida2010,Schreier2013,Bauer2012,Cornelissen2016,Liao2014,Basso2016,Mook2016,Nakata2017a}. These have been studied previously, but without accounting for their drift-mediated coupling to a nonequilibrium magnon chemical potential. We demonstrate that as regards the role of these mechanisms in nonlocal magnon transport, their leading order effect may be captured via a magnon drift velocity. Comparing the latter for these three representative mechanisms, we assess that temperature gradient should offer a good handle for influencing the spin propagation length in nonlocal magnon transport.

\section{Phenomenology of drift}\label{sec:phenomenology}

\begin{figure}[tbh]
	\begin{center}
		\includegraphics[width=85mm]{figure1}
		\caption{One-dimensional random walk~\cite{Fabian2007}. During one time step of the walk, particles in a bin of size $l$ may move to the right (left) bin with a probability $p_+$ ($p_-$). Their transport bears a drift contribution when $p_+ \neq p_-$.}
		\label{fig:randomwalk}
	\end{center}
\end{figure}

As compared to electronic spin transport~\cite{Fabian2007}, magnons constitute a platform with several qualitative distinctions as spin carriers. These differences include the bosonic, non-conserved nature of magnons as well as their carrying a scalar spin polarized along the direction of equilibrium magnetic order. We begin by considering the one-dimensional random walk~\cite{Fabian2007} of a large number of nonconserved particles to elucidate the requirements for emergence of drift. Dividing the space into bins with a small length $l$, there are $n(x,t)$ particles at a given time $t$ in the bin located at $x$. During one step of the random walk, which is assumed to take a small time $\tau$, the particles can do one of the following three things. They can jump to the right (left) bin with a probability of $p_+$ ($p_-$). Or they can disappear with probability $1 - p_+ - p_-$. Thus, the particles after one step in a bin at position $x$, $n(x,t+\tau)$, were at the adjacent bins before the step such that:
\begin{align}\label{eq:rand1}
n(x,t + \tau) & = p_+ n(x - l,t) + p_- n(x + l,t),
\end{align}
where the first term on the right hand side accounts for the particles that have arrived from the left bin, and the second term accounts for those arrived from the right bin. Employing Taylor expansion in~(\ref{eq:rand1}) and denoting $n(x,t)$ simply by $n$, we obtain
\begin{align}
n + \frac{\partial n}{\partial t}  \tau& = - \frac{\partial n}{\partial x} l \left( p_+ - p_- \right) + \frac{\partial^2 n}{\partial x^2} \frac{l^2}{2} (p_+ +  p_-) + (p_+ + p_-)n,
\end{align}
\begin{align}
\implies  \frac{\partial n}{\partial t} + \frac{\partial}{\partial x} \left( v_d n - D \frac{\partial n}{\partial x} \right) & = - \frac{n}{\tau_n}, \label{eq:cont}
\end{align}
where the final result takes the form of particle continuity equation~\cite{Fabian2007}. The current, given by the expression enclosed in brackets [(\ref{eq:cont})], includes a diffusive component parameterized via $D \equiv l^2 (p_+ + p_-)/ (2 \tau)$ and a drift contribution given in terms of the drift velocity $v_d \equiv l (p_+ - p_-) / \tau$. The right hand side of~(\ref{eq:cont}) accounts for particles disappearing with a time constant $\tau_n = \tau / (1 - p_+ -p_-) $. Here, we have assumed the particles to completely vanish at large enough times. In general, relaxation tends to bring the particle density to an equilibrium value~\cite{Kittel2004}. Equation (\ref{eq:cont}) shows that the drift velocity is a direct consequence of particles preferring to go toward one direction as compared to the other. This can be accomplished by breaking the spatial inversion symmetry from the {\em particles' perspective}, which is generally different from the full system Hamiltonian, as clarified further below.

When one considers electrons which are conserved~\cite{Fabian2007}, $p_+ + p_- = 1$ and $\tau_n \to \infty$, such that the sink term on the right hand side of~(\ref{eq:cont}) vanishes. Furthermore, the prototypical drift current in an electronic system results from an applied electric field~\cite{Fabian2007,Appelbaum2007,Huang2007,Kameno2014,Ingla-Aynes2016} such that the drift velocity is proportional to the applied electric field. This relation can be evaluated within the Drude model, for example, leading to Ohm's law. Employing this mechanism, a strong modulation of electronic spin propagation length has been demonstrated in various materials. From a theory perspective~\cite{Fabian2007}, it is often assumed that $p_+ - p_- \ll 1$, which further implies $v_d \ll l/\tau \sim v_{\mathrm{rms}}$, where $v_{\mathrm{rms}}$ is the root mean square velocity of the particles.

In uniformly ordered magnets, a homogeneous applied magnetic field typically does not break the spatial symmetry from the perspective of magnons. Even though it breaks the spatial symmetry for the spin system and consequently the magnetic ground state, the magnon Hamiltonian remains spatially invariant. This has motivated several authors to consider the magnetic field gradient as the driving force for magnon flow~\cite{Meier2003,Kosevich2013,Liao2014,Basso2016,Mook2016,Mook2018,Nakata2015,Nakata2017a}. This mechanism is similar to the case of electric field acting on electrons, which may be seen as the gradient of electric potential~\cite{Chen2005}, and will be addressed in Section~\ref{sec:real}. This is tantamount to breaking the spatial symmetry in real space. Second, we consider the magnon dispersion to bear a contribution antisymmetric in the wave-vector (Section~\ref{sec:reciprocal}). This is representative of symmetry breaking in the reciprocal space, and via the group velocity directionality. This mechanism is intricately related to chiral modes and enables a homogeneous magnetic field to influence the spatial symmetry of magnons~\cite{Gladii2016,An2013,Mook2016,Moon2013,Cortes-Ortuno2013,Schlitz2021,Yu2021}. Finally, we consider the possibility of spatial symmetry breaking by an incoherent property characterizing the system, such as temperature~\cite{Sanders1977,Xiao2010,Adachi2011,Uchida2010,Schreier2013,Bauer2012,Cornelissen2016,Liao2014,Basso2016,Mook2016,Nakata2017a}, in Section~\ref{sec:thermal}. But first, we establish the general role and manifestations of drift in nonlocal magnon transport experiments within a simplified, but rigorous, model in Section~\ref{sec:nonlocal}.

\section{Nonlocal magnon spin transport}\label{sec:nonlocal}

\begin{figure}[tbh]
	\begin{center}
		\includegraphics[width=90mm]{figure2}
		\caption{Nonequilibrium magnons, characterized by a nonzero chemical potential, are injected into a ferromagnetic insulator (yellow) by electronic spin accumulation generated in a heavy metal electrode (gray). These transport through the magnet and are detected by a separate heavy metal electrode as the magnon chemical potential at its location. Due to a pre-existing drift current (depicted via green arrows) in the magnet, the magnon propagation length bears a contribution proportional to the drift current [(\ref{eq:lp})] allowing for the former's control via the latter.}
		\label{fig:setup}
	\end{center}
\end{figure}

We now describe our general model for magnonic spin transport observed via electrical injection and detection of spin in a ferromagnetic insulator using the setup depicted in Figure~\ref{fig:setup}. Via the spin Hall effect~\cite{Hirsch1999,Sinova2015}, a charge current driven through the injector electrode generates spin accumulation at its interface with the magnet, which in turn injects magnons into the latter. These propagate in the magnet reaching detector electrode on the right, where they drive a spin current into the detector. Via inverse spin Hall effect~\cite{Saitoh2006,Sinova2015}, this is detected as a voltage under open circuit conditions. Thus, a charge current in the injector leads to a voltage in the detector mediated by magnonic spin transport in the magnet. The ratio of this detected voltage to the injected current is termed nonlocal magnetoresistance and is directly measured in experiments~\cite{Zhang2012,Cornelissen2015,Goennenwein2015,Cornelissen2016,Li2016}.

Focusing on the magnon propagation in the ferromagnetic insulator first, the transport can be formulated in terms of the magnon continuity, derived using the Boltzmann equation approach~\cite{Kittel2004,Chen2005,Cornelissen2016} in \ref{sec:formulate}:
\begin{align}
\frac{\partial n}{\partial t} + \pmb{\nabla}\cdot\pmb{j}_m & = - \frac{n - n_0}{\tau_m}, \label{eq:magcont}
\end{align}
where $\pmb{j}_m$ is the magnon current density, $\tau_m$ is the magnon decay time, and $n_0$ is the equilibrium magnon density. As detailed further in \ref{sec:formulate}, the relatively simple formulation of~(\ref{eq:magcont}) is enabled by the separation of magnon scattering time scales~\cite{Cornelissen2016}. The processes that conserve the spin and consequently the number of magnons are predominantly mediated by exchange interaction, which is the strongest energy scale in the magnet, and are fast~\cite{Akhiezer1968,Cornelissen2016}. We characterize them with a small phenomenological time $\tau$. The value of $\tau$ and the scattering processes that come to dominate it will depend on the situation under consideration. On the other hand, the magnon decay takes places via processes that do not conserve their number and that are mediated by weaker interactions, such as dipole-dipole interaction~\cite{Akhiezer1968,Cornelissen2016}. These are characterized by a larger time scale $\tau_m \gg \tau$. The situation is thus similar to the case of random walk considered in the preceding section.

Due to this hierarchy of time scales, primarily the nonzero magnon chemical potential characterizes the excess magnons (injected by a heavy metal, for example) and their transport in the magnet~\cite{Cornelissen2016}. Furthermore, due to a rapid thermalization without changing the number of magnons, the latter can be characterized by a common local temperature for the entire system that includes phonons. As a result of this, the magnon density time dependence \ak{can primarily be described via the chemical potential, as detailed further in \ref{sec:formulate}}:
\begin{align}\label{eq:mudot}
\frac{\partial n}{\partial t} & = \chi \frac{\partial \mu}{\partial t},
\end{align}
where the general form of $n(\pmb{r},t) = n_{0} + \chi \mu(\pmb{r},t)$ \ak{is obtained using the Boltzmann theory formulated in \ref{sec:formulate}} for the various specific cases considered in this work. Further, the magnon current density can be expressed in the following general form:
\begin{align}\label{eq:jgen}
\pmb{j}_m & = \pmb{j}_0 - \sigma_m \pmb{\nabla} \mu + \chi \pmb{v}_d \mu,
\end{align}
where $\pmb{j}_0$ is a spatially homogeneous contribution independent of $\mu$, $\sigma_m$ is the magnon conductivity~\cite{Cornelissen2016}, and $\pmb{v}_d$ becomes the drift velocity. \ak{The specific expressions for the magnon current density $\pmb{j}_m$ induced by different drives are obtained in different sections below using the formalism described in \ref{sec:formulate}.} Combining Eqs.~(\ref{eq:magcont})-(\ref{eq:jgen}), we obtain the equation governing magnon chemical potential and thus, transport:
\begin{align}\label{eq:chemcont}
\frac{\partial \mu}{\partial t} - D_m \nabla^2 \mu + \pmb{v}_d \cdot \pmb{\nabla} \mu & = - \frac{\mu}{\tau_m},
\end{align}
where $D_m = \sigma_m/\chi$ is the magnon diffusion constant. We treat~(\ref{eq:chemcont}) as the definition for drift velocity as the equation allows its direct interpretation in terms of its effect on magnon transport, as demonstrated below. In the following sections, we evaluate and compare $\pmb{v}_d$ under various situations hosting finite drift currents.

In order to capture the qualitative physics within a simplified analytic model~\cite{Kamra2020,Cornelissen2016}, we assume the magnetic layer to be thin and the device depicted in Figure~\ref{fig:setup} to be spatially invariant along the $z$-direction. With these assumptions, we may assume the magnon chemical potential to depend only on the $x$ coordinate making the equation to be solved [~(\ref{eq:chemcont})] one-dimensional. \ak{This approximation is tantamount to disregarding chemical potential and temperature variation in the direction perpendicular to the magnet/heavy metal interface. While being a good approximation for thin films, it breaks down when the magnetic layer thickness is comparable to the magnon diffusion length of few microns. Under those conditions, a two- or three-dimensional numerical modeling is necessary~\cite{Cornelissen2016}.} We further assume the injector and detector electrodes to be weakly coupled with the magnetic insulator layer, and the magnon drift velocity $\pmb{v}_d$ to be directed in the magnetic film plane. Under these circumstances, as detailed in \ref{sec:Rnl}, the magnon injection is accounted for via the boundary condition~\cite{Kamra2020}:
\begin{align}\label{eq:bc1}
- \left. \sigma_m \frac{\partial \mu}{\partial x} \right|_{x=0} & = j_{\mathrm{in}},
\end{align}
where we assume the injector to be located at $x = 0$, and $j_{\mathrm{in}}$ is proportional to the charge current driven through the injector electrode as detailed in \ref{sec:Rnl}. With these assumptions and in steady state, the solution to~(\ref{eq:chemcont}) for the range $x>0$ is obtained as:
\begin{align}
\mu(x) & = \frac{l_p j_{\mathrm{in}}}{\sigma_m} \exp \left( - \frac{x}{l_{p}} \right), \label{eq:muevol} \\
l_{p} & = \sqrt{\lambda_m^2 + \left( \frac{v_{dx} \tau_m}{2} \right)^2} + \frac{v_{dx} \tau_m}{2} \approx \lambda_m +  \frac{v_{dx} \tau_m}{2}, \label{eq:lp}
\end{align}
where $\lambda_m \equiv \sqrt{D_m \tau_m}$ is the magnon diffusion length, $v_{dx}$ is the $x$ component of the drift velocity, we assume $|v_{dx} \tau_m| \ll \lambda_m$ for simplicity, and we further required $\mu(x \to + \infty) \to 0$ in obtaining the above solution. Equation (\ref{eq:lp}) shows that the magnon propagation length $l_{p}$ bears a contribution from drift, which can be positive or negative depending on the sign of $v_{dx}$. Thus, the magnon propagation can be modulated via the drift~\cite{Schlitz2021}. Without loss of generality, we consider the drift to point along the $x$ axis in the rest of our analysis such that we may replace $v_{dx} \to v_d$.

Within our assumption of a weakly coupled detector electrode, as detailed in \ref{sec:Rnl}, the nonlocal voltage signal detected by the right heavy metal electrode is proportional to the magnon chemical potential at its location $x_d$~\cite{Kamra2020,Cornelissen2016}:
\begin{align}
\mu(x_d) & = \frac{l_p j_{\mathrm{in}}}{\sigma_m} \exp \left( - \frac{x_d}{l_{p}} \right), \\
   & \approx \frac{\lambda_m j_{\mathrm{in}}}{\sigma_m} \exp \left( - \frac{x_d}{\lambda_m} \right) \left( 1 + \frac{v_d \tau_m}{2 \lambda_m} + \frac{x_d v_d \tau_m}{2 \lambda_m^2} \right), \label{eq:muxd}
\end{align}
where we assumed $|x_d v_d \tau_m| \ll \lambda_m^2$ in addition to $|v_d \tau_m| \ll \lambda_m$ assumed already. Equation ~(\ref{eq:muxd}) shows that a positive drift velocity increases the signal detected by the right heavy metal electrode. The contribution of drift can be isolated experimentally by recording the dependence of this signal [(\ref{eq:muxd})] on handles, such as applied magnetic field direction~\cite{Schlitz2021} or temperature gradient magnitude, that influence the drift velocity.

In typical experiments, the heavy metal electrodes are coupled not so weakly to the magnetic insulator since the detected signal is directly proportional to the square of this coupling, quantified via the interfacial spin conductance~\cite{Cornelissen2016}. Under those conditions, the analysis of experimentally measured nonlocal magnetoresistance becomes tedious and simple analytic expressions are not available~\cite{Cornelissen2016}. Hence, while our analysis captures the qualitative physics well, it might become necessary to perform simulations for a comparison with experiments. Further, our thin-film one-dimensional model does not admit the possibility of different drifts at the two surfaces of the magnet. In case the drift current varies through the magnetic insulator thickness, the magnon chemical potential transport is more sensitive to the drift current close to the surface that is interfaced with the heavy metal electrodes. Such effects can be captured by solving the full 3-dimensional~(\ref{eq:chemcont}) and are beyond the scope of this work.

\section{Real space dependence of dispersion}\label{sec:real}

We now derive expressions for magnon current and the corresponding drift velocity considering a spatially dependent dispersion. An example of this situation is an applied magnetic field with its magnitude varying linearly in space. Such a drive has been considered by several authors~\cite{Meier2003,Kosevich2013,Liao2014,Basso2016,Mook2016,Mook2018,Nakata2015,Nakata2017a} previously using a broad range of analytic and numerical methods. Here, we follow the Boltzmann equation approach of Ref.~\cite{Liao2014}, in which the focus was on thermal transport of the magnons driven by the magnetic field gradient. Generalizing their methodology~\cite{Liao2014,Chen2005,Kittel2004} to include a nonzero magnon chemical potential~\cite{Cornelissen2016}, we obtain the desired expression for the magnon current and drift velocity.

In this approach, a WKB approximation is made and magnons are assumed to have an energy $\hbar \omega$ that depends on the spatial position: $\omega \equiv \omega(\pmb{r},\pmb{k}) = \omega_H(\pmb{r}) + \omega_0 + \beta k^2 \equiv \omega_H(\pmb{r}) + \omega_s(\pmb{k})$. Here, we consider the spatially dependent part to result from the Zeeman energy due to the applied magnetic field $H(\pmb{r}) \hat{\pmb{x}}$: $\omega_H(\pmb{r}) = |\gamma| \mu_0 H(\pmb{r})$, where $\gamma$ is the typically negative gyromagnetic ratio, and $\mu_0$ is the permeability of vacuum. The contribution $\omega_s = \omega_0 + \beta k^2$ results from anisotropy and exchange interaction. As outlined in \ref{sec:formulate}, the dependence of magnon current on the drives is obtained by solving the Boltzmann equation at short time scales corresponding to the time $\tau$. The magnon current becomes (\ref{sec:formulate}):
\begin{align}\label{eq:jm}
\pmb{j}_m & = \int_{\mathrm{BZ}} \frac{d^3k}{\left( 2 \pi \right)^3} \pmb{v}_g f(\pmb{r},\pmb{k}) ,
\end{align}
where $\pmb{v}_g = \pmb{\nabla}_{\pmb{k}} \omega = 2 \beta \pmb{k}$ is the group velocity, and $f(\pmb{r},\pmb{k})$ is the distribution function given in the relaxation time approximation by (\ref{sec:formulate})
\begin{align}\label{eq:fmaggrad}
f(\pmb{r},\pmb{k}) & = n_{B}(\hbar \omega - \mu) + \delta f(\pmb{r},\pmb{k}), \quad \mathrm{with} \\
 \delta f(\pmb{r},\pmb{k}) & =  - \tau \left. \frac{\partial n_{B}}{\partial \epsilon} \right|_{\hbar \omega - \mu} \pmb{v}_g \cdot \left( \hbar \pmb{\nabla} \omega_{H} - \pmb{\nabla} \mu  \right),
\end{align}
where $n_B(\epsilon) = 1/(\exp(\epsilon/(k_B T)) - 1)$ is the Bose distribution function with $k_B$ the Boltzmann constant and $T$ the temperature. Retaining only linear contributions, we obtain from Eqs.~(\ref{eq:jm}) and (\ref{eq:fmaggrad}):
\begin{align}\label{eq:jmmaggrad}
\pmb{j}_m & = \chi D_m |\gamma| \hbar \mu_0 \pmb{\nabla} H - \chi D_m \pmb{\nabla} \mu + \chi 2 \beta \tau |\gamma| \mu_0 \Gamma ~ \mu ~ \pmb{\nabla} H,
\end{align}
where
\begin{align}
\chi & \equiv  - \int_{\mathrm{BZ}} \frac{d^3k}{\left( 2 \pi \right)^3}  \left. \frac{\partial n_{B}}{\partial \epsilon} \right|_{\hbar \omega_s}, \label{eq:chi} \\
 D_m & \equiv - \frac{4 \beta^2 \tau}{\chi}  \int_{\mathrm{BZ}} \frac{d^3k}{\left( 2 \pi \right)^3}  \left. \frac{\partial n_{B}}{\partial \epsilon} \right|_{\hbar \omega_s} k_z^2 , \label{eq:Dm} \\
 \Gamma & \equiv \frac{2 \beta \hbar}{\chi}  \int_{\mathrm{BZ}} \frac{d^3k}{\left( 2 \pi \right)^3}  \left. \frac{\partial^2 n_{B}}{\partial \epsilon^2} \right|_{\hbar \omega_s} k_z^2 . \label{eq:Gamma}
\end{align}
A comparison of the magnon current expression thus obtained [(\ref{eq:jmmaggrad})] with its general form~(\ref{eq:jgen}) enables identification of the different contributions. Further, employing~(\ref{eq:jmmaggrad} in the magnon continuity equation (\ref{eq:magcont}) leads us to~(\ref{eq:chemcont}) with
\begin{align}\label{eq:vdmaggrad}
\pmb{v}_d & = 4 \beta \tau \Gamma |\gamma| \mu_0 \pmb{\nabla} H.
\end{align}
In obtaining our result in the form of~(\ref{eq:chemcont}), a small correction to $D_m$ has been disregarded. Furthermore, the drift velocity given by~(\ref{eq:vdmaggrad}) that enters the magnon continuity equation (\ref{eq:chemcont}) is larger by a factor of 2 compared to the drift velocity that enters the current density expression [(\ref{eq:jmmaggrad})]. This additional contribution results due to the magnetic field dependence of $D_m$ and the consequent term in the divergence of magnon current density.

Equation (\ref{eq:vdmaggrad}) is the main result of this section. \ak{We note that the smaller magnon scattering time $\tau$ determines the drift velocity [equation (\ref{eq:vdmaggrad})], instead of the magnon decay time $\tau_m$.} Among the various factors that influence drift velocity, only $\tau$ bears a substantial temperature dependence making low temperatures favorable for higher drift velocities. In order to estimate the latter at room temperature, we consider $\Gamma \approx 1$, $\tau = 1$ ps~\cite{Cornelissen2016}, $\hbar |\gamma|/ k_B = 1.3$ K/T~\cite{Liao2014}, $\hbar \beta = 8 \times 10^{-40}$ J$\mathrm{m}^2$~\cite{Cornelissen2016} and obtain $\pmb{v}_d \approx  ( 5 \times 10^{-6} ~\mathrm{m}^2/\mathrm{s} \mathrm{T} ) ~ \mu_0 \pmb{\nabla} H$. Here, magnon-phonon scattering is expected to dominate $\tau$ which is approximated as the inverse magnon-phonon scattering rate~\cite{Cornelissen2016}. Thus, rather large magnetic field gradients are required for even modest drift currents.

\section{Reciprocal space dependence of dispersion}\label{sec:reciprocal}

We now consider a mechanism for drift that emerges from spatial symmetry breaking in the reciprocal space. This ensues when the dispersion bears a contribution leading to the group velocity breaking the spatial symmetry~\cite{Nembach2015,Gladii2016,Mook2016,Moon2013,Cortes-Ortuno2013,Schlitz2021,Yu2021,Wang2020}. A prominent example of this are the chiral modes that live on the sample edges~\cite{Mook2014,Mohseni2019,Kim2016a,Owerre2016,Thingstad2019}. Such modes have previously been exploited in directional thermal transport~\cite{An2013}, for example. Their role in influencing the magnon chemical potential can thus also be anticipated. Here, we restrict our discussion to the thin film situation which is unable to distinguish between the two surfaces of the magnet, keeping in mind that transport dominated by one surface yields results similar to our analysis below.

We account for the spatial symmetry breaking in the reciprocal space by including a small antisymmetric contribution to the magnon dispersion $\omega(\pmb{k}) = \omega_s(\pmb{k}) + \omega_a(\pmb{k})$, such that $\omega_s(- \pmb{k}) = \omega_s(\pmb{k})$ and $\omega_a(- \pmb{k}) = - \omega_a(\pmb{k})$. Such contributions have been theoretically predicted and experimentally observed in chiral magnets and hybrids~\cite{Nembach2015,Cortes-Ortuno2013,Moon2013,Wang2020,Garst2017,Tokura2018}. The emergence of such a contribution due to the interfacial Dzyaloshinskii-Moriya interaction has been found to cause drift and the consequent control of magnon propagation length in recent nonlocal experiments~\cite{Schlitz2021}.

In our theoretical analysis here, we account for the antisymmetric contribution perturbatively i.e., we retain terms up to the first order in $\omega_a(\pmb{k})$ and assume that it does not alter the symmetric Brillouin zone of the material. The latter assumption is justifiable when $\omega_a(\pmb{k}) = \pmb{v}_{0} \cdot \pmb{k}$ is caused by a spatial symmetry breaking via an interface perpendicular to $\pmb{v}_0$~\cite{Nembach2015,Kim2016,Moon2013,Wang2020,Schlitz2021}. This is because an alteration of the spatial symmetry along a specific direction should not affect the Brillouin zone properties along orthogonal directions. However, this assumption and the following analysis need not be valid in chiral materials~\cite{Garst2017,Tokura2018} with bulk inversion symmetry breaking giving rise to $\omega_a(\pmb{k})$. An analysis of such materials will be carried out elsewhere.

The magnon current can be evaluated using~(\ref{eq:jm}) with the distribution function in the relaxation time approximation given by:
\begin{align}
f(\pmb{r},\pmb{k}) & = n_{B}(\hbar \omega_s + \hbar \omega_a - \mu) + \delta f(\pmb{r},\pmb{k}),
\end{align}
where
\begin{align}
n_{B}(\hbar \omega_s + \hbar \omega_a - \mu) & \approx  n_{B}(\hbar \omega_s) - \left. \frac{\partial n_{B}}{\partial \epsilon} \right|_{\hbar \omega_s} \mu + \hbar \omega_a \left( \left. \frac{\partial n_{B}}{\partial \epsilon} \right|_{\hbar \omega_s} - \left. \frac{\partial^2 n_{B}}{\partial \epsilon^2} \right|_{\hbar \omega_s} \mu  \right), \\
\delta f(\pmb{r},\pmb{k}) & \approx  - \tau \pmb{v}_g \cdot \pmb{\nabla} n_{B}(\hbar \omega_s + \hbar \omega_a - \mu) = - \tau \left. \frac{\partial n_{B}}{\partial \epsilon} \right|_{\hbar \omega - \mu} (\pmb{v}_s + \pmb{v}_{a})\cdot \pmb{\nabla} \mu,
\end{align}
where $\pmb{v}_{s,a} \equiv \pmb{\nabla}_{\pmb{k}} \omega_{s,a}(\pmb{k})$. Employing the two equations above in~(\ref{eq:jm}) and retaining the lowest order terms, we obtain the desired general expression for the magnon current given in~(\ref{eq:jgen}) with:
\begin{align}
\pmb{j}_0 & = \int_{\mathrm{BZ}} \frac{d^3k}{\left( 2 \pi \right)^3} \left[ n_{B}(\hbar \omega_s) \pmb{v}_a + \left. \frac{\partial n_{B}}{\partial \epsilon} \right|_{\hbar \omega_s} \hbar \omega_a \pmb{v}_s \right], \\
\sigma_m & = - \tau \int_{\mathrm{BZ}} \frac{d^3k}{\left( 2 \pi \right)^3}  \left. \frac{\partial n_{B}}{\partial \epsilon} \right|_{\hbar \omega_s} v_{sz}^2, \\
\chi \pmb{v}_d & = - \int_{\mathrm{BZ}} \frac{d^3k}{\left( 2 \pi \right)^3} \left[ \left. \frac{\partial n_{B}}{\partial \epsilon} \right|_{\hbar \omega_s} \pmb{v}_a + \left. \frac{\partial^2 n_{B}}{\partial^2 \epsilon} \right|_{\hbar \omega_s} \hbar \omega_a \pmb{v}_s  \right].
\end{align}
Considering $\omega_s(\pmb{k}) = \omega_0 + \beta k^2$ and $\omega_a(\pmb{k}) = \pmb{v}_0 \cdot \pmb{k}$, the expressions above are evaluated as:
\begin{align}
\pmb{j}_0 & = \pmb{v}_0 \left( n_0 - \frac{\chi \hbar D_m}{2 \beta \tau} \right), \\
\sigma_m & = \chi D_m,  \\
\pmb{v}_d & =  \pmb{v}_0 \left( 1 - \Gamma \right), \label{eq:vdv0}
\end{align}
where $\chi$, $D_m$, and $\Gamma$ have been defined previously in Eqs.~(\ref{eq:chi}) - (\ref{eq:Gamma}). Further, $n_0$ is the magnon density in equilibrium given by:
\begin{align}\label{eq:magdenasymm}
n_0 & = \int_{\mathrm{BZ}} \frac{d^3k}{\left( 2 \pi \right)^3} n_{B}(\hbar \omega_s) .
\end{align}
Equation (\ref{eq:vdv0}) is the desired expression for the drift velocity and constitutes the main result of this section. The contribution $\Gamma$ has been disregarded in the theoretical analysis of Ref.~\cite{Schlitz2021} and is significant.

One might consider an alternative approach. The $\omega_a(\pmb{k}) = \pmb{v}_0 \cdot \pmb{k}$ contribution considered in evaluating~(\ref{eq:vdv0}) effectively shifts the bottom of the parabolic dispersion away from $\pmb{k} = \pmb{0}$. Thus, one could redefine a new variable $\pmb{\tilde{k}}$ centered around the new dispersion minimum, thereby reducing the problem to the one without the linear-in-k contribution to the dispersion. This is however not allowed because the integration is over the first Brillouin zone [(\ref{eq:jm})]. Any change of variable necessitates modifying the integration domain in a consistent manner. Hence, it is convenient to not make a variable substitution and follow our method of separating even and odd contributions. Further, in contrast with charge currents, global nondissipative spin currents in equilibrium are allowed since spin-orbit coupling or similar effects render spin a non-conserved quantity (e.g., see Ref.~\cite{Chen2014}).

\begin{figure}[tb]
	\begin{center}
		\includegraphics[width=85mm]{figure3}
		\caption{Drift velocity vs.~temperature resulting from an asymmetric contribution $\pmb{v}_0 \cdot \pmb{k}$ to the magnon dispersion [(\ref{eq:vdv0})]. Magnon Debye temperature $T_D = 400$ K and $\hbar \omega_0 / k_B = 1$ K have been assumed. The dashed line indicates the asymptotic value provided in~(\ref{eq:vdv0app}).}
		\label{fig:drift_v0}
	\end{center}
\end{figure}

The ensuing drift velocity [(\ref{eq:vdv0})] has been plotted against temperature in Figure~\ref{fig:drift_v0}, where $\Gamma$ [(\ref{eq:Gamma})] has been evaluated assuming a spherical Brillouin zone with radius $k_{\mathrm{BZ}}$ defined in terms of the magnon Debye temperature $T_D$ assuming a single branch in the dispersion: $\hbar \beta k_{\mathrm{BZ}}^2 \equiv k_B T_{D}$. The low temperature limit of $\Gamma \to 1$, which corresponds to a vanishing drift velocity (Figure~\ref{fig:drift_v0}), has been corroborated via an analytic calculation. The high temperature limit of $\Gamma$ is evaluated as:
\begin{align}\label{eq:asymp}
\Gamma (T \to \infty) & \approx 1 - \frac{2}{3 t \arctan t - 3},
\end{align}
where $t \equiv \sqrt{k_B T_D/ \hbar \omega_0} \gg 1$. As shown by the numerically generated plot of Figure~\ref{fig:drift_v0}, this limit is nearly attained for temperatures comparable to $T_D$ and the drift velocity observed at room temperature is close to this value:
\begin{align}
\pmb{v}_d & \approx   \frac{2}{3 t \arctan t - 3} ~ \pmb{v}_0. \label{eq:vdv0app}
\end{align}
Thus, for yttrium iron garnet with the lowest dispersion branch $T_D$ of about 400 K~\cite{Cherepanov1993,Cornelissen2016,Barker2016}, the drift velocity at room temperature is expected to be two orders of magnitude smaller than $v_0$. With $v_0 \sim 10$ m/s~\cite{Wang2020,Schlitz2021}, $v_d \sim 0.1$ m/s is still large compared to what we estimate in the previous section from a reasonable magnetic field gradient. Thus, for the mechanism under consideration, high temperatures are favorable for drift.

\section{Thermal drive}\label{sec:thermal}

The mechanisms for spatial symmetry breaking, and consequently drift, considered above may be classified as ``coherent'' since they stem from altering a single-particle property - the energy. Now, we consider an incoherent mechanism in the form of temperature gradient. A spatial symmetry breaking by a thermodynamic property, such as temperature, describing the ensemble could also lead to drift. Our consideration of thermal gradient for effecting drift is encouraged by the success of thermally driven spin currents in a wide range of magnetic materials and hybrids~\cite{Uchida2010,Bauer2012,Xiao2010,Adachi2011,Uchida2008,Jaworski2010,Adachi2013,Wu2016,Seki2015,Hirobe2017,Rezende2016,Ohnuma2013,Geprags2016,Rezende2014}. However, our considered influence of thermally generated magnon drift on electrically injected and detected magnon transport is qualitatively different from the spin Seebeck effect. For example, in our considerations, no voltage is detected by the normal metal electrode if nonequilibrium magnons are not injected first [e.g., see~(\ref{eq:muevol})], irrespective of the thermal gradient. Further, with the aim of examining drift velocity in the presence of more than one mechanism causing it, we consider the same magnon dispersion $\omega = \omega_s + \omega_a = \omega_0 + \beta k^2 + \pmb{v}_0 \cdot \pmb{k}$, as we did in the preceding section.

The magnon current can be evaluated via~(\ref{eq:jm}) employing the usual relaxation time approximation, as described in \ref{sec:formulate} and used in the previous sections. Furthermore, we continue to assume the magnon and phonon temperatures to be the same, due to the magnon-phonon thermalization time being small ($\sim 1$ ps)~\cite{Cornelissen2016}. In the present evaluation, the equilibrium distribution $f_0(\pmb{r},\pmb{k})$ is assumed to be the Bose distribution function with a spatially homogeneous temperature. In evaluating the magnon current driven by a constant temperature gradient, we assume the deviation of temperature from its assumed equilibrium spatially homogeneous value to be small, and substitute this deviation to zero in our final result. After lengthy calculations and retaining only the lowest order terms, we obtain magnon current density in the form of~(\ref{eq:jgen}) with:
\begin{align}
\pmb{j}_0 & = \pmb{v}_0 \left( n_0 - \frac{\chi \hbar D_m}{2 \beta \tau} \right) - \alpha \pmb{\nabla} T, \label{eq:j0therm} \\
\alpha & \equiv   - \frac{4 \beta^2 \hbar \tau}{T} \int_{\mathrm{BZ}} \frac{d^3k}{\left( 2 \pi \right)^3}  \left. \frac{\partial n_{B}}{\partial \epsilon} \right|_{\hbar \omega_s} k_z^2 \omega_s, \label{eq:alpha} \\
\pmb{v}_d & = \pmb{v}_0 \left( 1 - \Gamma \right) - \Lambda \pmb{\nabla} T, \label{eq:vdtemp} \\
\Lambda & \equiv \frac{4 \beta^2 \hbar \tau}{T \chi}  \int_{\mathrm{BZ}} \frac{d^3k}{\left( 2 \pi \right)^3}  \left. \frac{\partial^2 n_{B}}{\partial \epsilon^2} \right|_{\hbar \omega_s} k_z^2 \omega_s . \label{eq:lambda}
\end{align}
Employing the current expression thus obtained in the magnon continuity equation (\ref{eq:magcont}), we obtain the chemical potential dynamics in the form of~(\ref{eq:chemcont}) with the drift velocity given by~(\ref{eq:vdtemp}).

In obtaining the results above [Eqs.~(\ref{eq:j0therm})-(\ref{eq:lambda})], we limit ourselves to linear response considering $\pmb{\nabla}T$ and $\pmb{\nabla} \mu$ as the linear drives. The drift term $\propto \mu \pmb{\nabla}T$ is captured adequately in this approximation. In considering nonlocal magnon transport, we are only interested in the transport of magnons that have been injected externally. This means that in our magnon continuity equation, we should only have terms which vanish in the limit $\mu \to 0$. Our linear response results above naturally yield only such terms. If one goes beyond linear response, terms which do not vanish in the limit $\mu \to 0$ and act as source or sink of magnons can be expected. However, in the ongoing analysis, these are neither needed nor can they be faithfully evaluated.

\begin{figure}[tb]
	\begin{center}
		\includegraphics[width=85mm]{figure4}
		\caption{Temperature dependence of the proportionality factor $\Lambda$ that relates drift velocity to the thermal gradient [Eqs.(\ref{eq:vdtemp}) and (\ref{eq:lambda})]. $T_D = 400$ K and $\hbar \omega_0 / k_B = 1$ K have been assumed.}
		\label{fig:Lambda}
	\end{center}
\end{figure}

Equations (\ref{eq:vdtemp}) and (\ref{eq:lambda}) are the main result of the present section and show that the effects of multiple drift mechanisms simply add up in the drift velocity expression. Our explicit demonstration of this here could be anticipated on the basis of linear response principles. The parameter $\Lambda$ [(\ref{eq:lambda})] determines the drift velocity caused by the applied thermal gradient and has been plotted in Figure~\ref{fig:Lambda}. Since $\Lambda$ scales as $1/T$, it decreases with temperature making low temperatures favorable for thermally-induced magnon drift. Furthermore, $\tau$ in the expression for $\Lambda$ [(\ref{eq:lambda})] is not determined by magnon-phonon scattering, since we assume the magnon and phonon temperatures to be identical. The time scale $\tau$ would have been related to magnon-phonon scattering if we would consider a thermal gradient in magnon temperature alone while the phonons would remain in equilibrium. Since we consider a common temperature gradient for both subsystems, $\tau$ is a relatively long time scale governed by scattering with impurities, among others. The value $\tau \sim 1$ ns has been employed previously~\cite{Liao2014} in obtaining results consistent with experiments on yttrium iron garnet, and we adapt this value here. Thus, employing $\tau = 1$ ns, $\hbar \beta = 8\cdot 10^{-40}$ J$\mathrm{m^2}$~\cite{Cornelissen2016}, $T_D = 400$ K~\cite{Cornelissen2016,Cherepanov1993,Barker2016}, $\hbar \omega_0/k_B = 1$ K~\cite{Cornelissen2016}, we obtain $\pmb{v}_d =  (2 \times 10^{-4} ~ \mathrm{m}^2/\mathrm{K} \mathrm{s}) ~ \pmb{\nabla}T$ at room temperature. Thus, drift velocities comparable to those observed in recent experiments~\cite{Schlitz2021} are expected for thermal gradients $\sim 1$ K/mm. In contrast with magnetic field, large temperature gradients are regularly and conveniently generated in labs due to the localized nature of heat generation in solid state systems~\cite{Jaworski2010,Uchida2010,Uchida2008}. Equipped with the above analysis, we expect temperature gradients to offer a convenient and effective handle of magnonic drift velocity and thus, the magnon propagation length.

\section{Conclusion}\label{sec:conclusion}

Inspired by the corresponding role in electronic spin transport~\cite{Fabian2007} and recent experiments on magnons~\cite{Schlitz2021}, we have theoretically examined the role of drift currents in controlling the magnonic spin propagation length, as observed in nonlocal experiments. Employing a phenomenological description based on the random walk model~\cite{Fabian2007}, we established that a magnon drift current requires spatial symmetry breaking in the magnonic description. We further found that it modulates the magnon propagation length, which can be a direct experimental signature, as established in recent experiments~\cite{Schlitz2021}. Employing the Boltzmann approach, we evaluated the magnon drift velocity caused by three representative symmetry breaking mechanisms - magnetic field gradient, magnon chirality, and thermal gradient. Using experimentally measured parameters (which vary considerably among different reports), we estimate these drives to potentially result in an increasing magnitude of the drift velocity, with thermal drive potentially offering the largest values.

Our analysis here assumes a quasi-continuous magnon dispersion and evaluates the transport coefficients, especially the drift velocity, in terms of the Brillouin zone sum over all magnon modes. While providing useful general relations, the present endeavor will benefit from a more microscopic and numerical analysis in the future, where a spin Hamiltonian is instead the starting point. This will be especially important for examining the case of asymmetric contribution to the magnon dispersion with regards to its spatial dependencies and the Brillouin zone rigidity. On the experimental side, our analysis anticipates and paves the way for employing thermal drive, and the consequent drift currents, in controlling the magnon propagation length in nonlocal magnonic spin transport experiments.

\section*{Acknowledgments}
We thank Sebastian Goennenwein, Bart van Wees, and Gerrit Bauer for valuable discussions. We acknowledge financial support from the Spanish Ministry for Science and Innovation -- AEI Grant CEX2018-000805-M (through the ``Maria de Maeztu'' Programme for Units of Excellence in R\&D) and grant PID2020-114880GB-I00. Sebastián de-la-Peña is grateful to Instituto Universitario de Ciencia de Materiales Nicolás Cabrera for one of its Research Awards for Physics Students 2021.

redpajama_set_name: RedPajamaArXiv


The needs for the St. Agnes Pantry Food Drive collection have changed.
As a separate ministry from the St. Ignatius and St. Agnes Community Food Pantry housed at St. Agnes, the St. Agnes Pantry Food Drive collection now requests foods in easy-to-open packaging for snack bags that will be distributed to people living on the streets or who don't have access to a kitchen.
-Boxed or canned juice, e.g. V8.
-Vienna sausage or other protein packaged in a pull-top container.
-Fruit cups or apple sauce.
-Protein bars or other healthy snacks.
Please place your contributions in the baskets located at the church entrances at any of the weekend Masses.


text:
typedef struct temptag
{
	uchar dsdir[8];
	uchar ds1820[8];
	uchar ds2423[8];
	uchar ds2401[8][8];
	uchar ctrl[16];
   int   weather_a;
   int   weather_b;
   int   found_dir;
   int   found_1820;
   int   found_2423;
   int   found_2401;
   int   north;
} WeatherStruct;

// local function prototypes
int FindSetupWeather(int portnum, WeatherStruct *wet);
int SetupWet(int portnum, WeatherStruct *wet, int nor);
int ReadWet(int portnum, WeatherStruct *wet, float *temp, int *dir, double *revol);
int GetDir(int portnum, WeatherStruct *wet);
int TrueDir(int portnum, WeatherStruct *wet);
int ParseData(char *inbuf, int insize, uchar *outbuf, int maxsize);

redpajama_set_name: RedPajamaGithub


Yesterday marked the official beginning of my 44th year and I had a fantastic day celebrating it on the golf course with my twin brother Jimmy, my father Don, and my son Patrick. While we were checking in with the starter, I saw some guys with various cameras set up right by the 9th green which is parallel to the first teebox. Having done a fair amount of "man on the street" interviewing on behalf of my clients, I had a hunch that they were seeking some testimonials or sound bytes from "real people" about the game. My suspicions were confirmed when the interviewer introduced himself as a representative of the USGA (United States Golf Association for the uninitiated) and asked if we wouldn't mind talking to him about our relationship with the game. He later admitted that we were of particular interest because we represented three generations of men; I was tempted to introduce dad as my older brother, but I didn't think they'd buy it.
The big question area he kept circling back to revolved around why we play the game. Jimmy spoke about having time to himself out in the fresh air and dad spoke about his introduction to the game through the business world and how he used it to bond with customers (I used to joke that he was the chief golf officer of American Express). Patrick talked about getting his love for the game from me, which begs the question, why do I play?
Part of my answer is reflected in Patrick's — I play golf because my father introduced it to me at a young age. Oftentimes he would come home from playing a round on a weekend day and then take us to the range where he would show Jimmy and me how to swing. While his passion became mine, that wasn't enough to keep me in the game. While I agree with my brother that it is great to spend some time outside in the fresh air playing a game, for me, it's more than that.
I used to consider golf a collection of shots that amounted to nothing more than a round, but now it's bigger than that/ It represents the chance to master (and remaster) a skill — defining an objective and planning on how to meet it. In golf, this translates to being able to put your ball where you want it on its journey to its final destination (the hole). Not only that, but doing it in as few tries as possible — and improving every time. Golf has become a metaphor for what I value in life — the ability to put thought (or a desire) into action and to do it with a greater degree of excellence every time.
Off the course, this means growing my business. I'm self employed and unless I'm successful in winning projects from my competition, my family won't eat. The stakes are high. As with lining up a shot on the golf course, I have to identify the right solutions to help my clients address real business challenges. Once I win the opportunity to work with a client, I have to execute flawlessly so that they come back to play another round with me.
the course and in the boardroom, what's ultimately important is the outcome and how adversity was overcome.
As you can see, golf to me is a bit more than an escape or a way to develop customer relationships — it is a metaphor for life. If feel so strongly about this that I used golf to drive the narrative of Winning Streak, my third novel. While it's not about golf per se, it is about adversity and how we overcome adversity and loss in our lives. You can buy it here.
The week leading up to my birthday started with what I thought was going to be a great deal of adversity. For Christmas, I bought my daughter Grace tickets to see one of her favorite performers – Shawn Mendes. Opening for Shawn was another one of her favorites, Charlie Puth. Now I'm a rocker and modern pop music isn't my thing. On top of that, I promised she could take two friends along and that we'd stay the night in Boston (It should be known that I assumed Gracie would pick her brother and sister to go with, but that wasn't the case). Having to take on the responsibility of other kids is not something I embrace without at least a little hesitation.
In the weeks leading up to the concert, I didn't exactly hide my lack of enthusiasm for this event but something funny happened when I was at the venue with Grace and her friends; I started to get into it. I saw a few other dads who had the look in their faces as if they drew the short straw that night and I saw how much it bothered their daughters. I decided then and there that I would let my excitement level rise – and it did to the point where Grace told me I was embarrassing her. "Why cant you be like other dads?" came out of her mouth more than once.
I knew I had a choice — sulk because I didn't like where I was or who I was going to see, or feed off the energy from Grace and 18,000 other screaming girls (and let me tell you, 18,000 girls can do a lot of screaming). I am convinced the girl sitting next to me (not one of Grace's crew) actually peed in her pants when Shawn took the stage. Instead of peeing, my Gracie actually started to cry when Shawn took to the mic. Speaking of which, if you've never done something with your daughter that she was so into that she starts to cry because she's so happy, you haven't lived (you see, crying I'm okay with, but I draw the line at public urination).
If there's one lesson in this, which at this point feels more like a rant than a reflection, is that life is full of adversity but it's what we do about that adversity that defines us. Oftentimes, its our attitude that makes all the difference. On the course we can choose to slam our club down in reaction to a bad shot or we can take a deep breath, evaluate what we did wrong, and learn from it (and hopefully recover). In a professional setting we can either react calmly to a hurdle we are faced with, or we can start yelling and screaming about what put it in our way (what do you think will have the better outcome?). And in Boston's TD Garden we can sulk like all the other parents who do not share the same musical taste as their children, or we can embrace it and learn to live vicariously through the pure joy in our children's eyes. What would make us better at parenting?


text:
Q: Javascript - zip and sum variable number of arrays in single expression The answer to Javascript equivalent of Python's zip function shows a neat way of taking any number of arrays, and "zipping" them into a merged array in a single statement.
zip= rows=>rows[0].map((_,c)=>rows.map(row=>row[c]))

This question Javascript - Sum two arrays in single iteration shows a similar idea, but summing the entries as they're zipped up.
I'm wondering how to combine the two techniques - so given an unknown number of arrays:
[
  [1,2,3],
  [1,2,3],
  [1,2,3]
]

... the result is [3, 6, 9], ie the sum of the first elements, the second and so forth. For the sake of simplicity, assume each array contains the same number of items.

A: First transpose the arrays, so the columns become rows and viceaversa. After that simply call the reduce function.
The first version of the code is mostly typescript for brevity. The second version is JavaScript.
Note that ES5 map and reduce functions are only available on IE9 and higher.

var numbers = [[1,2,3],[1,2,3],[1,2,3]]

// TypeScript

var colSums = numbers[0].map(function(col, i) {
  return numbers.map((row) => row[i]).reduce((a,b) => a + b );
});

// JavaScript

/*var colSums = numbers[0].map(function(col, i) {
  return numbers.map(function(row) {
    return row[i];
  }).reduce(function(a,b) {
    return a + b;
  });
});*/
document.getElementById("col-sums").innerHTML = colSums;

A: I think I have it - this answer was helpful - we can extend the original zipping method thus:
zip = rows => rows[0].map((_,c) => rows.map(row=>row[c]).reduce((a,b) => a+b,0))

A: No need for map, map, reduce, two maps will get you there:
Quick Demo
var m = [
  [1,2,3],
  [1,2,3],
  [1,2,3]
];

var total = m.map(function(arr, i) {
  var count = 0;
  return arr.map(function(el, idx) {
    return count += m[idx][i];
  })
}).pop()

A: Similar to other answers, it just doesn't have to be so complicated:

numbers = [[1,2,3],[1,2,3],[1,2,3]];

var result = numbers[0].map(function(_, i) {
  return numbers.reduce(function(prev, row) {
    return row[i] + prev;
  }, 0);
});

console.log(result);

redpajama_set_name: RedPajamaStackExchange


An ultra-fine, lightweight powder that sets makeup with an illuminating finish that evens skin tone and blurs the look of imperfections while hydrating the skin and minimising shine throughout the day.
Gently tap closed container to fill dispense product into the tray. Dip brush in the powder, gently tapping off excess product and dust over the face, layer for desired coverage.
I-035455	Phyto Pigment Flawless Finishing Powder Juice Beauty An ultra-fine, lightweight powder that sets makeup with an illuminating finish that evens skin tone and blurs the look of imperfections while hydrating the skin and minimising shine throughout the day.


If sound barriers are built along a portion of the U.S. 250 bypass as part of the so-called Best Buy ramp, a Charlottesville design committee wants the Virginia Department of Transportation to keep them as simple as possible.
"[They] need to be as plain as possible and include vegetation to the extent possible," said Rachel Lloyd, chair of the city's PLACE Design Task Force. The group was created in 2012 to advise City Council on the aesthetics of public infrastructure.
The $17.2 million project was first conceived more than a decade ago as part of a larger study to reduce traffic congestion at the interchange of U.S. 29 and U.S. 250. VDOT officials hope to advertise the project for construction in November.
The plan also includes an additional south lane on U.S. 29 between Hydraulic Road and the interchange, but Thursday's discussion at the PLACE group's meeting was restricted to the sound walls that will line both sides of U.S. 250.
"Federal Highway Administration regulations require there be a sound wall installed along the 250 bypass as part of this project," said Jim Tolbert, the city's director of neighborhood development services.
The walls would vary in height depending on the location, but would be as high as 25 feet in some places.
"The only way it would not be installed is if enough of the property owners opt out and don't want sound walls," Tolbert added.
VDOT has not yet formally asked affected residents whether they want to have the walls built, and more than half need to support the project, Tolbert said.
"We're proceeding with the presumption that we're going to install the sound walls as presented," Cubbage said.
With the project soon to go to bid, Tolbert wanted the PLACE committee to weigh in on the aesthetics. They were shown a number of different visual treatments that could be applied to the walls.
"Each of them offers a different pattern that we could include in the contract or we can leave it as a standard brushed finish," Cubbage said.
However, PLACE members were not satisfied by the various treatments.
However, VDOT's noise abatement program manager said they are cautious when installing vegetation on sound walls.
PLACE committee members were more concerned that homeowners and renters know how they will be affected.
"They should be made aware of the shading effects and the lack of air movement that's going to occur," Mark Watson said.
"I feel like the questions people are asking about how best to communicate the design and engineering information to neighbors is probably more critical to us at this point than picking between [designs]," Lloyd said.
A design public hearing for the project was held in November 2012. PLACE members also asked if another public meeting could be held, though there is nothing in state or federal law that would compel VDOT to do so.
The Best Buy project is now included in a funded and approved package of transportation projects currently being planned for the U.S. 29 corridor.
Philip Shucet, a former VDOT commissioner who is overseeing implementation of the projects, told an advisory panel that he wants the Best Buy project to be completed no later than July 31, 2016.


text:
Preacher: Scott Williamson (176), Jonathan Blake (94), Ricky Rew (62), Daniel Hatfield (38), Paul Wheeler (34), Stuart Conway (19), Les Maybury (19), 1st Sunday Team (15), Doug Crisp (12), Elizabeth Ajayi (7), Joe Hayden (7), Mike Collins (6), Colin Brown (5), Caroline Kerry (4), Claire King (4), Anton Machacek (4), First Sunday Team (4), Vanessa Redbond (4), Brian Riley (4), Connor Winston (3), Christina Hatfield (3), Nick Lear (2), Gavin Calver (2), Rev. David Shosanya (2), Scott Williamson / Les Maybury (2), Childrens Nativity (2), Phil Wright (2), Various (1), Paul Wheeler; (1), Linda Harrison (1), Claire King/Ricky Rew (1), Jane Guest (1), Richard King (1), BMS Action Team (Mozambique) (1), BMS Action Team (Andrew, Alex, (1), Jonathan Blake / Scott William (1), Claire King & Stuart Conway (1), Ricky Rew/Jonathan Blake (1), Testimony (1), Dr Nathan & Kristen Henson (1), Jack Hooper (1), Lewis Powis (1), Elizabeth (1), Rev Stuart Elmes (1), James from Action Team (1), BMS Uganda Action Team (1), RBC Youth (1), Anthony Comber (1), Heather and Mike Collins (1), Sue Comber (1), Emilie Radford (1), Steve Cooper (1), Dianne Tidball (1), Gill Hayden (1), Scott Williamson & Daniel Hatf (1), Benjamin Francis (1), Martyn Dolan / Andy Redbond (1), Andrew Kerry (1), Don Cooper & Scott William (1), Joy Clark (1), BMS TEAM (1), Scott Williamson & Jonathan Bl (1), David McCahon (1), John Pike & Jonathan Blake (1), Scott Williamson & John Pike (1), Ivan (1), Peter Dunn (1), Laura-Lee Lovering (1), Rowland Clear (1), Andy Howard (1), Trevor Campbell (1), Mike Colins and Andy Redbond (1), Faith G / Val P / Sheila B (1), Heather Collins (1), Ian Childs (1), Pete Everett (1). … (70 more)
Book: Genesis (8), Exodus (2), Deuteronomy (1), Joshua (2), Judges (1), Ruth (1), 1 Samuel (1), 1 Kings (4), Nehemiah (9), Esther (2), Psalm (6), Proverbs (16), Isaiah (6), Jeremiah (1), Daniel (10), Hosea (1), Joel (1), Amos (1), Jonah (6), Zechariah (1), Matthew (33), Mark (5), Luke (16), John (23), Acts (27), Romans (9), 1 Corinthians (10), 2 Corinthians (4), Galatians (16), Ephesians (14), Philippians (1), Colossians (9), 2 Thessalonians (1), 2 Timothy (5), Hebrews (3), James (2), 1 Peter (3), 1 John (7), Revelation (8). … (30 more)
Series: Discovering Jesus (2), Alpha (1), Christmas 2020 (3), Just Like Us (8), Empowered by the Holy Spirit (14), Faith for Lifes Journey (11), Gods work in the lives of His people (Telling our stories) (5), Telling Our Stories (3), Understanding Gods Purpose for the Church (9), Jesus the Gift of hope (1), Authentic Christianity (5), Joshua (1), The Path (5), Encouragement for the journey of faith (7), Lessons from series (1), Lessons From (1), Standalone Messages (3), BMS Action Team (2), Palm Sunday (2), Embracing Gods design for the Church (9), LENT (3), All Age Service (5), Jesus is Enough (5), Devotion to God (6), Advent Love and Forgiveness (1), Go in the Strength you have (1), No Longer Slaves (8), Book of James (5), Promises of God (3), The Promises of God (2), Mark10 v13-16 (1), Jesus said 'I AM' (5), I am (3), BMS Uganda Action Team (2), All Age Signed Service (9), Desiring God (5), Seven Dangers Facing the Church (9), Holy Week (2), Praise & Prayer (12), One (8), A City on a Hill (5), City on a hill (2), Pride and Humility (1), Family Service (4), The King is Coming (1), School of Prayer (4), Emotionally Healthy Spirituality (7), The School of Prayer (5), Emotionally Healthy Spiritually (3), God is.... (2), Words of Christ on the Cross (1), Surprise the World: habits of an everyday disciple (5), Theology of New Expressions (3), New Expressions (1), Refreshing your Soul (5), Pentecost (1), All is Grace (6), What is Hope? (1), The Great Commission (1), Daniel (1), What I love about Jesus (15), The Book of Daniel (14), Advent (5), Luke 12:48-Indian Team Update (1), Spiritual Gifts (5), The hard sayings of Jesus (10), Galatians 1 v3 -9 (1), Security (1), Hebrews 10 v 19-25 (1), Prayer (3), First Sunday 2 (1), Guest Speaker (9), Table Talks (4), Maundy Thursday (1), Jonah (5), Acts (25), Discipleship Pathway (15), 2 Corinthians (1), Proverbs (16), 1 Peter (2), Nehemiah (12), Matthew (1), Colossians (2), Luke (1), 2 Timothy (7), Baptism (6), Mission (8), Parables of Jesus (7), Beatitudes (9), Numbers (1), Easter (11), John (4), Philippians (8), All Together (15), New Beginnings (2), Early Morning Communion (4), 1 John (6), Psalms (7), Communion service (9), Christmas (13), Letters of James (3), The Armour of God (5), Minor Prophets (4), Practical Parables (5), First Sunday (25), Other (27). … (97 more)
Service: Sunday Morning (304), Sunday Evening (248), Midweek Meeting (14), Early Morning Service (13), Special event (6).
Date: 2001 (1), 2014 (30), 2015 (105), 2016 (117), 2017 (95), 2018 (86), 2019 (87), 2020 (61), 2021 (3)
Passion in Action
2 Thessalonians 22:47-53 (Part of the Just Like Us series).
Preached by Elizabeth Ajayi on 08/11/2020 (Sunday Morning).
Messing Up
John 18:15-27 (Part of the Just Like Us series).
Right Motives, Wrong Outcomes
Matthew 16:21-23 (Part of the Just Like Us series).
Preached by Les Maybury on 25/10/2020 (Sunday Morning).
Public Declaration of Faith
Preached by Stuart Conway on 18/10/2020 (Sunday Morning).
Responding to God's Call
Luke 5:1-11 (Part of the Just Like Us series).
Preached by Paul Wheeler on 11/10/2020 (Sunday Morning).
Holy Spirit- Tongues & Interpretation
1 Corinthians 14:1-19 (Part of the Empowered by the Holy Spirit series).
Preached by Jonathan Blake on 04/10/2020 (Sunday Morning).
Holy Spirit- Discerning the Spirits - 1 Cor. 12-1, 4-6
1 Kings 22:1-8 (Part of the Empowered by the Holy Spirit series).
Holy Spirit - Faith, Healing & Miracles - 1 Cor. 12:7-11
Luke 17:11-19 (Part of the Empowered by the Holy Spirit series).
Holy Spirit - Prophecy (1 Cor 14:1-5)
Holy Spirit - Words of Knowledge & Wisdom


text:
Blogging.la
Lizard people dude. Seriously.
Posted on May 31, 2006 by Sean Bonner
Sheriffs and CCWs and Cronies, Oh My!
There's an interesting back and forth going on between Jim March and Glen Craig (Retired Sheriff, Sacramento County) in regards to the current CCW policies in CA. While they are specifically talking about a situation in Sacramento, it's state law that allows it and elected Sheriffs that decide how to enforce it. Last year I posted a link to a video debate between LA's Sheriff Baca and OC's Sheriff Carona that shows exactly how different the law allows policies to be. In Jim March's reply to Glen Craig's note, Jim mentions LA and OC specifically in reference to situations that look a bit shady (the core of the discussion is speculation that only wealthy campaign contributors have a chance of getting a CCW license in Sacramento, and how this is mirrored statewide). Here's the snip of that section:
How is it that when Sheriff Baca of LA set up an "executive reserves program" stocked with 20 major campaign contributors, and within a year one had chased a neighbor down the street in his underwear and another "upstanding citizen" laundered a quarter mil through Israel of all places and ran guns into Mexico.
How did the sole CCW holder in the city of Oakland end up being a serial sexual molester with personal connections to the mayor? That's a 100% failure rate.
Or how about the latest from Orange County? Sheriff Carona has a sweet little program arming rich Los Angeles folks (now that Baca dumped 'em?) by issuing them a joke reservist status and one of same such "cops" was found connected to (and supplying guns for) the scam artist that wrecked the stolen Ferrari doing 160mph DUI.
As I mentioned last week, the current situation that let's one person decide on a whim who should and shouldn't be able to carry a gun in public begs for corruption, where as a policy closer matching how drivers licenses are distributed (if you apply and meet a set of requirements you will be approved, regardless of how much is in your bank account or who you know) is much more fair. Again, it's important to stress that the person calling the shots on this is elected by the people in the county. Sheriff Baca is on the ballot for reelection next week – there are 4 other candidates running against him. While none of the candidates have discussed this topic openly – Ken Masse, who has a blog, seems to have impressed some people with his take on it. Point being, know who you are voting for and what they are supporting.
On a site note, I'd really like to hear from some LASD people (or LAPD people for that matter) on this topic, even if just on the last question in Jim's note:
What's going on now is a freakshow. What kind of morale problem does this send through a department, when the whole staff figures the boss is on the take? Can I as a citizen trust a cop/deputy who is willing to work for such an agency, or do I have to look at every single member of such a department as a potential gang member with a badge?
UPDATE: Please see the comments for a note from Paul Jernigan – pro-CCW candidate for Sheriff.
CategoriesLA, Rants
2 Replies to "Sheriffs and CCWs and Cronies, Oh My!"
paul jernigan says:
I am Paul Jernigan, candidate for Los Angeles County Sheriff.
I do take a stand regarding CCWs and it is posted at my website at http://www.jerniganforsheriff.com
I am a firm believer in the right to own and bear arms. As Sheriff, I will issue CCWs to anybody that passes a background check and a gun safety class.
I was a street cop during the 1992 riots, and in the middle of fighing them. We were so overwhelmed by the rioters, the public had to defend themselves without our help for about 24 hours. Those with guns did not get robbed and their businesses did not burn.
Thank you, and please vote June 6, 2006,
Paul L. Jernigan Jr.
sean bonner says:
Thanks very much for your comment Paul! I'm checking out your site now…
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text:
Coronavirus breakthroughs in vaccine…
Your Tax Dollars
Coronavirus breakthroughs in vaccine development, inhaler therapy reported
FILE – In this Wednesday, June 24, 2020 file photo, a volunteer receives a COVID-19 test vaccine injection developed at the University of Oxford in Britain, at the Chris Hani Baragwanath hospital in Soweto, Johannesburg, South Africa. People on six continents are testing experimental shots as the race for a COVID-19 vaccine enters a defining summer, with even bigger studies poised to prove if any leading candidate really works – and possibly offer the public a reality check. (AP Photo/Siphiwe Sibeko)
By Alexi Cohan | Boston Herald
PUBLISHED: July 20, 2020 at 6:51 p.m. | UPDATED: July 21, 2020 at 8:06 a.m.
Coronavirus breakthroughs in vaccine development and an inhaler therapy were separately reported Monday as the United States continues to see record-breaking spikes in cases of the deadly disease.
A coronavirus vaccine created by scientists at the University of Oxford in England triggered strong immune responses and neutralizing antibodies, according to a study published Monday.
"It's a really important milestone to put into the public domain our findings on the safety and immune responses to this vaccine in the first group of people that we vaccinated," said Sarah Gilbert, University of Oxford professor and project lead on the study.
The vaccine provoked an immune response within 14 days of vaccination and an antibody response within 28 days, according to the study.
The participants had levels of neutralizing antibodies, which have been suggested by researchers as important for protection against the virus.
Those responses were strongest after a booster shot, with 100% of participants' blood having neutralizing activity against the coronavirus.
"Vaccines are absolutely the way out of the pandemic and this is a really important moment because it shows that we can make the robust immune responses which we hope will relate to protection in the future, " said Andrew Pollard, chief investigator of the University of Oxford study.
During the trial, more than 1,000 healthy adult volunteers got the vaccine and no serious health impacts were reported.
The University of Oxford is working with the United Kingdom-based global biopharmaceutical company AstraZeneca for the further development, large-scale manufacture and potential distribution of the COVID-19 vaccine.
In a separate announcement out of the UK, an inhaled formulation of an anti-inflammatory therapy used in COVID-19 patients was shown to lower the risk of developing a severe case of the disease, according to an announcement from the company Synairgen, which makes the treatment.
Richard Marsden, CEO of Synairgen said in a statement, "We are all delighted with the trial results announced today, which showed that SNG001 greatly reduced the number of hospitalised COVID-19 patients who progressed from 'requiring oxygen' to 'requiring ventilation.' "
Patients that received the formulation of inhaled interferon beta in a trial had a 79% lower risk of developing severe disease and were more than twice as likely to recover from the coronavirus than the placebo group, according to results presented Monday.
Marsden said patients who got the SNG001 treatment could resume everyday activities and reported reduced breathlessness.
"This assessment of SNG001 in COVID-19 patients could signal a major breakthrough in the treatment of hospitalised COVID-19 patients," said Marsden.
Alexi Cohan | Reporter
Alexi Cohan is a general assignment reporter covering local news and government as well as health and medicine stories. Alexi is from Springfield, Massachusetts and attended college at Hofstra University in New York where she majored in journalism and Spanish. Alexi's professional experience encompasses print, television and radio at NY1, CNN en Español, 88.7FM WRHU and The Republican newspaper. She enjoys making connections with the community she covers and imploring others to use journalism as a tool to stay informed and engaged.
Follow Alexi Cohan @lexcohan
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HAYARI Paris IN HOLLYWOOD FOR THE OSCARS !! 7 April 2014
HAYARI Paris in Hollywood for the Oscars!!
The week running up to the Oscars' ceremony is always a busy time for Nabil HAYARI, as stars and celebrities look for the most somptuous gowns to wear on the red carpet, and invitations to attend the most prestigious parties keep coming in.
Nabil Hayari et Afoma Eguh Okafor attending the Hellman&Walters' "Salute to the Stars" party.
On February 27th, 2014, Bob Hellman and Richard Walters were excited to announce that BiteSizeTV, the first online television network, with live studios in Hollywood, would be partnering with the 4th Hellman and Walter's Annual "Salute to the Stars" Oscar after-party, benefiting The Actors Fund.
Recognized by Variety, The Hollywood Reporter and CNN as one of the top Oscar events to attend in 2014, "Salute to the Stars" took over the rooftop at the luxury W Hollywood Hotel on March 2, 2014. The star-studded, red carpet event featured the variety band, TODDSPLANET with special guests including Taylor Hicks.
The "Night of 100 Stars", LA's premiere awards night Gala, was THE event that a few lucky people could gain access too. This party had stars galore, in fact 100's of stars were there, with actors like Richard Dreyfuss, Jacqueline Bisset, Harry Hamlin, Stephanie Powers all being past guests.
The stars also stepped out for Elton John's "Annual Oscars Viewing Party" to benefit his AIDS Foundation (EJAF) in West Hollywood.
This year's event co-chairs were Bill and Tani Austin, Johnny and Edwina Barbis, Joseph W. Blount, Jim Carrey, Chris Colfer, John Demsey, Judi Dench, Greg Gorman, Tim Hanlon and Anthony Klatt, Neil Patrick Harris and David Burtka, Diana Jenkins, Quincy Jones, Nicole Kidman and Keith Urban, Billie Jean King and Ilana Kloss, Heidi Klum, Ryan Kwanten, Fred Latsko, Shelley Lazar, Sandra Lee, Jared Leto, Andra Liemandt, Eric and Janet McCormack, Joseph A. McMillan, Jr., Sharon and Ozzy Osbourne, Anna Paquin and Stephen Moyer, Katy Perry, Tyler Perry, Pablo and Nathalie Salame, Caroline Scheufele, Bryan Singer, Sharon Stone, Steve Tisch, Steven Tyler, and John Waters.
Dawn Christie, wearing HAYARI Couture Paris, Bob Degadillo, Kris Jenner, Khloe Kardashian, Kourtney Kardashian and Kim Kardashian attend the 22nd Annual Elton John AIDS Foundation Academy Awards viewing party with Chopard at the City of West Hollywood Park on March 2, 2014 in West Hollywood, California. (Photo by Stefanie Keenan/Getty Images for Chopard) | Stefanie Keenan via Getty Images
The 15th Annual Oscar Viewing Party to benefit Children Uniting Nations took place on March 2nd 2014. This annual event has been listed as one of the 3 best Oscar parties and proceeds benefit Children Uniting Nations (CUN) and its programs for at-risk children.
It was a fabulous, sensational star-studded evening on the night of March 2nd, 2014, as various members of the Entertainment industry and celebrities gathered at the home of the founder Daphna Edwards Ziman in Beverly Hills for a Private Oscar Party event and Silent Auction.
Among some of the celebrities in attendance at the party that evening included famous Melanie Mar and American fashion model and actress Kimmarie Johnson, both in HAYARI Couture Paris Italian model Fabio Lanzoni, former Heavyweight Boxing Champion of the World Mike Tyson who is now turned comedian, French couture designer Nabil Hayari and Legendary Screen Actor and Musician Jeff Goldblum—who's band went on to play at the event later on in the evening.
Post Oscars Laucheon reception at the French Residence on March 3rd 2014
Just like last year, the French Consulate organised a post-Oscars Luncheon Reception at the French Residence, to congratulate French nominees and Oscar winners. Nabil Hayari, Hélène Segara, Laurent Witz, Alexandre Desplat,… were amongst the many French celebrities attending the famous event.
March 10th 2014, Hollywood's brightest stars hit the red carpet to attend the 86th Academy Awards nominee luncheon at The Beverly Hilton Hotel. Lupita Nyong'o, nominated for best supporting actress for "12 Years a Slave", Leonardo DiCaprio, a best actor nominee for "The Wolf of Wall Street", Sandra Bullock, nominated for best actress for "Gravity", Amy Adams, a best actress nominee for "American Hustle", Bradley Cooper, a best supporting actor nominee for "American Hustle", Julie Delpy, nominated for best adapted screenplay for "Before Midnight" and many others attended the event.
France was well represented at this year' s Academy Awards ceremony, with films competing in four categories:
Ernest & Celestine by Benjamin Renner, Vincent Patar, & Stéphane Aubier
The Missing Picture by Rithy Panh (for Cambodia), a French majority co-production
The Great Beauty by Paolo Sorrentino (for Italy), a French minority co-production
Best Short Film (Live Action)
Just Before Losing Everything by Xavier Legrand
Best Short Film (Animated)
Mr Hublot by Laurent Witz & Alexandre Espigares, a Franco-Luxembourg co-production
Julie Delpy is nominated in the Best Adapted Screenplay category (along with Ethan Hawke and Richard Linklater) for Before Midnight.
Bruno Delbonnel is a nominee for Best Cinematography for Inside Llewyn Davis
Alexandre Desplat will compete for the Best Original Music award for Philomena
Pierre Coffin and the entire MacGuff studio are nominated for Despicable Me 2 in the Best Animated Feature Film category