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Human Capital and Workforce Development
Workforce Investment
Workforce Policy
Service Providers to Low-Income Communities Face Challenges of Their Own
Low-income individuals and communities are feeling the brunt of job losses due to the pandemic. At the same time, organizations providing support services to that population are facing their own challenges. Partners Update explores southeastern organizations' sentiments from a national survey.
Household Financial Well-Being
Amid the COVID-19 Crisis, a Tale of Two Southeastern Cities
Congress passed the CARES Act and other legislation to help workers who have lost their jobs during the pandemic. Partners Update considers a case study of a hypothetical laid-off restaurant worker in Birmingham and Miami and the potential financial assistance he'd receive in each city.
A Fresh Look at Opportunity Occupations
The Center for Workforce and Economic Opportunity has updated its Opportunity Occupations Monitor data tool, which tracks trends in opportunity employment across the country. Partners Update discusses the tool's new features.
Measure of the wage growth of individuals. It is constructed using microdata from the Current Population Survey (CPS), and is the median percent change in the hourly wage of individuals observed 12 months apart.
Microbusinesses
How Do Firms Respond to Hiring Difficulties?
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Opportunity Occupations: Well-Paying Jobs for Middle-Skill Workers
What opportunities and decent-paying jobs exist for workers who don't have a college degree? This article gives an overview of recent Fed research on the topic.
An Eye on the Future: A Discussion about the Long-term Care Insurance Market
The Economy Matters podcast talks to Atlanta Fed economists about the long-term care insurance market.
Beige Book: Labor Market Tightness Reaching Entry-Level Jobs
Atlanta Fed business contacts have a mostly positive outlook on economic growth in the region. Economy Matters summarizes the part of the Beige Book reporting on economic conditions in the Southeast.
The Wherefores and Whys of Wages
After an extended period of relative stagnation, wages have been showing signs of growth. This episode of the Economy Matters podcast discusses recent wage trends and how the Atlanta Fed views wage behavior.
Beige Book Finds Optimism, Ongoing Hiring Challenges
Economy Matters article offers highlights of the Atlanta Fed's portion of the Beige Book.
Identifying Opportunity Occupations in the Southeast
The brochure examines the types and share of opportunity occupations—jobs for middle-skill workers that pay at or above the national median wage—in all Sixth District states. It also depicts returns to education across the Southeast.
Where Will Opportunity Knock? A Discussion of Opportunity Occupations
In an era when education's importance in the employment sector has steadily increased, what role do well-paying jobs that don't require a college degree play? An episode of the Economy Matters podcast talks to some Atlanta Fed experts.
The Labor Market Distributions Spider Chart is designed to allow monitoring of broad labor market developments by comparing current conditions to those in up to two earlier time periods that the user selects.
eBook: Developing Career-Based Training
This eBook examines various approaches to establishing technical and career-based training and the importance of building out the skills needed for the workforce in today's increasingly complex and rapidly changing global economy.
Uneven Opportunity: Exploring Employers' Educational Preferences for Middle-Skills Jobs
The Federal Reserve Banks of Atlanta and Philadelphia investigate the factors that contribute to employer requirements of a bachelor's degree for four key opportunity occupations.
Uneven Opportunity: Variation in Employers' Educational Preferences for Middle-Skills Jobs
New Philadelphia and Atlanta Fed research explores why employer preferences for bachelor's degrees for the most prevalent opportunity occupations differ significantly between metro areas. Partners Update summarizes the findings.
The Developing State of Workforce Development
An evolving economy demands workers with evolving skill sets, and training employees to meet new employment demands is an ongoing challenge. The episode discusses trends in workforce development in the Southeast as well as nationally.
eBook: Models for Labor Market Intermediaries
This eBook explores the role of community and economic development organizations in workforce development and the importance of fostering and facilitating partnerships to address local workforce challenges.
Identifying Opportunity Occupations in the Nation's Largest Metropolitan Economies
The report identifies good-paying jobs in the 100 largest U.S. metro areas for workers who have less than a four-year college degree. The Federal Reserve Banks of Atlanta, Cleveland, and Philadelphia collaborated on the findings. Full report (8 MB) | Infographic (392 KB)
Transforming U.S. Workforce Development Policies for the 21st Century
The book explores how new policies and practice can meet the changing needs of workers, businesses, and their communities. The Atlanta and Kansas City Feds and Rutgers' Heldrich Center for Workforce Development collaborated on the book, which has contributions from over 65 leading scholars and practitioners engaged in workforce development.
The Soft Skills Gap
In listening sessions with the Atlanta Fed, workforce training providers noted the lack of soft skills in some workers. Those skills can be roughly divided into essential and workplace skills, and this Partners Update article discusses each set of skills.
Microenterprises Raise the Floor and Build a Ladder
One outcome of the recent recession is that rural poverty rates are the highest since the mid-1980s. Mil Duncan, founding director of the University of New Hampshire's Carsey Institute, discusses the issues facing the rural poor in an Economic Development podcast episode.
Small Business and the Modern Workplace
What are the challenges facing small business after the Great Recession? Ty Barksdale of Sutton Bank and Jake Rouch of Erie Regional Chamber and Growth Partnership describe demands of the current workplace, including that workers be adaptable, collaborative, agile, and entrepreneurial.
Can the Jobs Gap Be Filled through Temporary Public-sector Positions?
Philip Harvey, professor of law and economics at Rutgers University, discusses how his proposed direct job creation program would create temporary public-sector jobs, and in the process, help reduce unemployment.
Trash to Treasure: Turning Waste into Jobs
Instead of sending waste to landfills, a municipal approach that prioritizes the reuse, recycling, and remanufacture of materials can provide a range of new jobs. Georgia Tech's Nancey Green Leigh discusses how to create jobs from the waste diversion process.
Retrofitting Institutions: Feeding Job Growth with Energy Hogs
Satya Rhodes-Conway and James Irwin, senior associates at the Center on Wisconsin Strategy, discuss how retrofitting public and institutional buildings spurs job creation in the real estate sector while reducing building operating costs.
The Doctor Is In: Economic Development Strategies in Health Care
The health care sector has been an important source of new jobs in this economy. Dr. Ricardo Azziz, president of Georgia Health Sciences University, discusses the importance of the sector to the economic well-being of communities and how its growth can help catalyze economic development.
Self-employment as Economic Development Strategy: What Does It Mean For Metro and Nonmetro Counties in the Southeastern United States?
New research suggests that self-employment is becoming an important solution to unemployment in the Southeast, especially in rural areas. But why are there different outcomes for urban and rural areas? And what are the implications for economic developers and policymakers?
New Economy, New Roles: Economic Development Organizations and Jobs
Economic development organizations must develop and execute job creation programs in today's difficult economy, even as their budgets are reduced. Denny Coleman, president and CEO of the St. Louis County Economic Council, discusses how local organizations can still add to the quantity and quality of local jobs.
Not Your Father's Factory Job: Manufacturing and Economic Development
Jay Moon, president and CEO of the Mississippi Manufacturers Association, discusses the increasingly technical and specialized skills needed to support advanced manufacturing. These skills, he says, are creating a greater focus on working with business, industry, and educational partners to develop a better-skilled workforce.
Small Things Really Matter: The Important Role of Microenterprise in Job Creation
Microenterprises, which employ about 20 percent of the U.S. private-sector workforce, have been especially important since the recent recession. Connie Evans, president and CEO of the Association for Enterprise Opportunity, discusses how economic developers can grow local jobs by supporting microenterprises.
The Job Hunt: New Clues for Small Business Job Creation
Newly available data provide fresh insights into employment in the small business sector. Brian Headd, economist in the Small Business Administration's Office of Advocacy, explores the changing relationship of small business to jobs.
Who Will Treat the Sick? Emerging Trends in the Hospital Based Workforce
Hospitals and their satellite operations are facing human capital frictions as the public demands the latest treatments in the most upgraded facilities and as they prepare to respond to new legislation. Dr. Stephen Newman, chief operating officer with Tenet Healthcare Corp., discusses these workforce challenges and opportunities.
Fact or Fallacy: Can Self Employment Improve Economic Opportunities for Low Skilled Workers?
For some low-skilled workers, self-employment appears to be the best opportunity to improve their earnings, but is it? Dr. Magnus Lofstrom, research fellow with the Public Policy Institute of California, discusses whether self-employment improves the earning power of low-skilled workers as well as economic development policies that local and state governments could consider to help this vulnerable population.
Center for Workforce and Economic Opportunity (CWEO)


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Hungary introduces a total ban on tobacco advertising
T Szilágyi
Health 21 Hungarian Foundation; http://health21.hungary.globalink.org
Correspondence to;
Tibor T Szilágyi MD, c/o Department of Public Health & community Medicine, University of Sydney, NSW 2006, Australia;
tibors{at}health.usyd.edu.au
Hungary has introduced a total ban on direct and indirect advertising for tobacco products
advertising ban
http://dx.doi.org/10.1136/tc.11.1.79
Although comprehensive tobacco control policy has yet to be adopted in Hungary, a legal framework for tobacco control is in place. The most important regulations on tobacco issues include: the 1997 Act on Advertising,1 amended by the 2001 Act on Advertising2; the Act on the Protection of Non-Smokers and Some Rules of Consumption and Trade of Tobacco Products3 (smoke-free environments, rules of purchasing tobacco products, minimum age for purchase and smoking), in force since November 1999; and the 36/1996 Interministerial Decree on packaging, warning labels and harmful substance content of cigarettes.
On 19 December 2000 Hungarian tobacco control advocates achieved a glorious victory over the tobacco industry when the Hungarian Parliament voted for an amendment of the 1997 Act on Advertising, which only forbade "tobacco advertising targeted at children and youth", billboards located within 200 m from educational or health establishments, and screening of tobacco ads before 8 pm in cinemas. The amendment introduced a total ban on direct and indirect advertising for tobacco products to take effect by 1 July 2001 for print media and by 1 January 2002 for outdoor posters and billboards.
Despite the general jubilation of tobacco control advocates, this success must not be taken as anything more than a victory in a very important battle, with few doubting that the war still continues. The tobacco industry's disappointment and frustration over events it was unable to influence will force it to dig new tactics from deep inside its international post-ban kitbag to challenge and circumvent the newly introduced measure. Zsolt Jamniczky, PR manager of Reemtsma, the third biggest tobacco company in Hungary, blubbed: "The Parliament accepted this bill and we have to adjust ourselves to it, but we are not happy. The timing is not very good." The "timing" he referred to was undoubtedly the rude interruption in the industry's marketing success which saw smoking prevalence in Hungary increase by 25% among secondary school students between 1995-99,4 with women's smoking rising by more than one third between 1986 and 2000.5,6
This total ban simply restored the 1978 decree of the Ministry of Internal Affairs which also banned all forms of tobacco advertising. The fall of the Berlin Wall and the transition to the market economy offered an excellent opportunity for transnational tobacco companies to jump on the free marketing bandwagon and invade the new market. The new investors immediately recognised the ad ban would severely hamper their ability to attract new consumers. The industry which had told journalists how important "conformance to laws"7 is for them, disregarded and violated the 1978 regulation as this Philip Morris document clearly states: " . . .competition has taken a very liberal approach in interpreting the law and has conducted massive billboard and similar campaigns . . . some of our marketing activities have been investigated and resulted in a $200,000 fine."8 Nonetheless, they were eager to change this situation: "In Hungary, we will seek through direct lobbying and action with third party allies to amend obsolete tobacco advertising legislation..."9
And they were successful in doing so. The tobacco and advertising industry, with the help of some servile representatives of the then ruling socialist government, succeeded in hastening the birth of the very liberal Act on Advertising in 1997.10 Young Democrats—now governing in Hungary—championed a stricter act but they were defeated by the ruling socialist party which had had many visible and invisible links to the tobacco manufacturers. The socialist government also tried to delay parliamentary debate of a bill aimed at protecting the rights of non-smokers, while tobacco control advocates and the then health minister, also a socialist, strongly lobbied for the bill. When the government was led by a chain smoker prime minister, who believed "smoking is a question of strength of will . . . nowadays, when smokers are really pursued you need more will-power to keep yourself to it",11 it was little wonder that his government did not find itself "committed enough" to harm the tobacco industry.
The adoption of this very liberal law, which allowed tobacco advertising in press, cinemas, theatres and on outdoor posters (figs 1, 2, and 3), resulted in the spread of campaigns often targeted at women (fig 1) and youth. Cigarettes were promoted as "friends in everyday life" (fig 2). This situation, along with the introduction of a new European Union (EU) Directive (EC 98/43) on tobacco advertising and sponsorship, energised Hungarian tobacco control advocates. Mr Lajos Pákozdi, an elder statesman in the fight against tobacco, took the lead by approaching the Hungarian Court of Constitution. He argued that tobacco advertising severely endangered the right to health of Hungarians and encouraged children to take up smoking. The court's verdict in November 2000 was ambiguous: on the one part it stated that "with the promulgation of the already in force regulation on tobacco advertisements the government acquitted its duty in protecting life and health. A total ban in tobacco advertising cannot be deduced from the Hungarian Constitution".12 However, it did not exclude the introduction of stricter regulation, if the government considered it necessary.
With the anticipated annulment of the EU advertising directive in October 2001, the Hungarian Ministry of Economics immediately removed the passages on tobacco marketing from its proposal submitted to the Parliament. The Health 21 Hungarian Foundation mobilised the tobacco control community, convening more than 20 representatives from government based agencies, non-governmental organisations, and the Parliament to take a common stand for much stricter regulation of tobacco promotion. The Foundation helped two MPs develop and submit amendments on further restrictions in tobacco advertising. A newsletter was distributed to MPs and to members of the Parliamentary Committee for Health and Social Affairs as well as to media representatives. Just before the deadline for submitting amendments to the advertising bill Mr Mihály Babák, MP of the ruling party of Young Democrats, submitted his amendment asking for regulation of promotion of tobacco products as strict as the aborted EU Directive. A letter, signed by all the participants of the forum, was sent immediately to all 386 members of the Hungarian Parliament asking to vote in the affirmative for the amendment. It seemed that the letter writing campaign achieved its goal. As Mr Babák put it later in an interview13: "If somebody voted against, he or she must have considered this question from other aspects or he cast his vote wrongly". A few days later, on 19 December 2001, the entire advertising act, including the total ban of direct and indirect tobacco advertising, was passed by the Parliament.
Mr Babák stressed that his main argument for the preparation of this submission was to keep the industry away from children: "It is time to start influencing public opinion and make smoking and its advertising unacceptable; children and youth should not be taken in by the messages communicated by tobacco companies: while smoking, the sky is always blue and the air is clean. Smoking is a dirty thing, which takes tar into the lungs of people. The industry is trying to reach new markets so tobacco advertising clearly aims at children and youth. And the individuals of these target groups are taken in since they are not able to take into account all consequences of smoking".
Similar to decision makers' claims in other countries14 the influence of tobacco control advocates and that of patients' rights organisations were also of great interest to Mr Babák when he took action. Tobacco control advocates should understand that the help of an MP of the ruling party could be more useful for them than an initiative coming from the opposition. Mr Babák put it this way: "I would not say that an amendment coming from the government party is always better, but we have the necessary background institutions which are at our disposal if submissions need to be revised professionally, and perhaps the Government prefers suggestions made by its own representatives."
Péter Dávid, external relations manager at Philip Morris Hungary, said: "I am very disappointed by the law because the Hungarian Government has decided to introduce it without prior consultation". Single amendments do not need to be the subject of formal consultation in Hungary. The industry was unprepared for the change. Timing is crucial. As Mr Babák stated: " . . .there was a tactical step to introduce it [his submission] later, when the tobacco industry would not have any opportunity to remove it. The shorter the time is for external attacks the greater the success in the Parliament. If you proceed in this way than the lobby does not have time enough to overrun all the parliamentarians. If the submission had been introduced earlier it would not have been passed."
Advocates, however, must not be satisfied and feel relieved, even if a new law is passed by the Parliament. All events must be followed continuously and carefully because "accidents" may happen later, especially if the industry's lobbying machinery is activated. In Hungary, the bill comes into force when it is signed by the President. Six pro-tobacco industry organisations, including the Advertising Self-Regulatory Body and the Association of Hungarian Publishers, sent in a petition to the Hungarian President Ferenc Mádl trying to persuade him not to sign the law. On 2 January 2001 the President's Office called upon Mr Pákozdi to review once again the possible roles and impacts on health of the new legislation. The outcome of the discussion was favourable to pro-health advocates: on 4 January 2001 the new law was proclaimed. The Hungarian media and our public places are now free of deceptive tobacco advertisements. Never ceasing vigilance is further needed as the tobacco industry maximally exploits the current weaknesses of the advertising regulations.15
Hungarian tobacco advertising campaigns were often targeted at women. Photo: Figyelo.
The slogan in this poster says: "Your friend in everyday life." Photo courtesy of Health 21 Hungarian Foundation.
Advertisements even exploited seasonal events, not always in a respectful way to women. Photo courtesy of Health 21 Hungarian Foundation.
1997, évi LVIII. törvény a gazdasági reklámtevékenységrôl. (Act on Economical Advertising Activities No. LVIII/1997). URL: http://www.complex.hu/kzldat/T9700058.HTM/MUN_2.HTM#kagy1 (in Hungarian)
2001, évi I. törvény a gazdasági reklámtevékenységrôl szóló 1997. évi LVIII. törvény módosításáról. (Act No. I/2001 amending the Act No. LVIII/1997 on Economical Advertising Activities). URL: http://www.complex.hu/kzldat/T0100001.HTM/MUN_2.HTM#kagy1 (in Hungarian)
1999, évi XLII. törvény a nemdohányzók védelmérôl és a dohánytermékek fogyasztásának, forgalmazásának egyes szabályairól (Act on the Protection of Non-smokers and Some Rules of Consumption and Trade of Tobacco Products No. XLII/1999). URL: http://www.complex.hu/kzldat/T9900042.HTM/MUN_2.HTM#kagy1 (in Hungarian)
Anon. Prevalence of cigarette smoking among secondary school students – Budapest, Hungary, 1995 and 1999. MMWR Morb Mortal Wkly Rep2000;49;438–41.
Central Statistical Office. Health Behaviour Survey, 1986.
Health Development Research Institute. Report on the National Health Behaviour Survey, April 2001. URL: http://www.gallup.hu/olef/gyors.html (in Hungarian).
Interview given by József Gábor, President of the Board of Directors of V-Tabak Ltd, the only Hungarian-owned tobacco company. Észak-Magyarország (Northern Hungary), 3 July 2001 (in Hungarian).
Philip Morris, 1994. OB Presentation on Central Europe, New York. 17 November 1993. Bates No. 2500108030. URL: http://www.pmdocs.com/getallimg.asp?if=avpidx&DOCID=2500107969/8065, p 31.
Philip Morris. Regional corporate affairs, summary of objectives, undated, Bates No. 2500070176. URL: http://www.pmdocs.com/getallimg.asp?if=avpidx&DOCID=2500070154/0218 (go to 2500070176).
"A dohányon vett parlament" (Parliament bought on baccy). Kukabúvár 1998;4:No2. URL: http://www.kukabuvar.hu/kb12/kb12_28.html
Anon. Interview given by the former Hungarian socialist Prime Minister Gyula Horn to the women magazine "Story", June 2000 (in Hungarian).
Moldoványi: Alkotmányos a dohányreklám. (Tobacco advertising is constitutional.) Magyar Nemzet, 2 November 2000:4. URL: http://www.magyarnemzet.com/news/fullstory.php/aid/12573.html (In Hungarian)
Our guest: Mihály Babák. Filter – Tobacco Advocacy Newsletter for Central and Eastern European Countries. June 30, 2001;1(2):4. URL: http://health21.hungary.globalink.org/filteronline
Montini T, Bero LA. Policy makers' perspectives on tobacco control advocates' roles in regulation development. Tobacco Control2001;10:218–24.
Fraser T. Phasing out point-of-sale advertising in New Zealand. Tobacco Control1998;7:82–4.
Hungary: tobacco ads forced back inside
Tibor Szilagyi
Tobacco Control 2004; 13 8-8 Published Online First: 25 Feb 2004.

redpajama_set_name: RedPajamaCommonCrawl


text:
Vanda Scaravelli
By Phil Catalfo , Aug 28, 2007
The daughter of artistic Italian parents, wife of a professor of philosophy, and an accomplished pianist, Vanda Scaravelli was accustomed throughout her life to meeting creative artists, intellectuals, and literati. The Indian philosopher J. Krishnamurti came to stay at the Scaravelli's villa overlooking Florence every year. When Scaravelli's husband died suddenly after World War II, she soon began spending summers with her children at a chalet in Switzerland, where she hosted Krishnamurti during his lectures there. B. K. S. Iyengar would come every morning to teach him yoga; he introduced Scaravelli, then in her 40s, to the ancient discipline, and "a new life came into my body." Thus began her ongoing exploration of what she called allegrezza, "the intelligent heart."
From T. K. V. Desikachar she learned breath awareness; she later formulated her own approach to yoga (in which "you become intelligent and at the same time you are happy") and began to teach others. Her book Awakening the Spine (Harper San Francisco, 1995) became a classic. Since her death in 1999, at age 91, several teachers have carried on her work, most notably Toronto-based Esther Myers. "I practice because it is natural for me to practice," she told Myers in a 1996 YJ interview. "There is no other reason.
The Longest Goodbye
The 2002 Karma Yoga Awards
Eknath Easwaran
Neem Karoli Baba (Maharajji)


In this blog we are walking through how to improve performance of application using Yourkit profiler it is helpful for both Tester and Developers.
Your Kit is big achievement in the evolution of the profiling tools. It is intelligent tools for profiling java , .net and ( JVM support languages) based applications.
It is often important to check memory usage and memory used per process on servers so that resources do not fall short and users are able to access the server. It is very effective for any application.
Out of Memory occurs when jvm cannot allocate object because it is out of memory.
Due to these problems our application leads to serious overall system performance degradation.
Heap Memory shows Java heap statistics.In this we can easily see individual pools or all pools together.Java uses the heap as the storage for Java objects.
Non-Heap Memory shows the non-heap memory statistics. Java uses the non-heap memory to store loaded classes and other meta-data. You can see individual pools or all pools together.
Classes shows how the number of loaded classes changed in time, and the total number of unloaded classes.
Object Allocation Recording graph shows the number of objects created per second.
Here you see the current memory allocations and number of objects has been created and size reserved.
CPU tab shows CPU consumption statistics. It is available when you are connected to the profiled application.
In this tab we are able to catch all the statistics performance at one place e.g CPU, Memory etc.
Using this we can improve performance of our application and make it effictive.
I hope this blog shows you what you can do with YourKit java profiler.


This semester, I am freelancing for The College Tourist, the student blogging website that I interned with in the fall! For my first article, I put together the ultimate packing list for Coachella. Check it out!


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7 edition of Exploring Philip Pullman"s His Dark Materials found in the catalog.
Exploring Philip Pullman"s His Dark Materials
An Unauthorized Adventure Through The Golden Compass, The Subtle Knife, and The Amber Spyglass (His Dark Materials)
by Lois Gresh
Published October 30, 2007 by St. Martin"s Griffin .
English literature: literary criticism,
Juvenile Nonfiction,
Literature - Classics / Criticism,
Children: Young Adult (Gr. 7-9),
Children"s Literature - General,
Reference - General,
Regional, Ethnic, Genre, Specific Subject,
Science Fiction & Fantasy,
Juvenile Nonfiction / Reference / General,
Literary Criticism & Collections,
Fantasy fiction, English,
History and criticism,
Juvenile literature,
Young adult fiction, English
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Get this from a library. Shedding light on His dark materials: exploring hidden spiritual themes in Philip Pullman's popular series. [Kurt D Bruner; Jim Ware] -- Unlike authors such as J.R.R.
Tolkien and C.S. Lewis, Pullman writes from an intentionally anti-Christian perspective. As the authors explore Pullman's themes, characters, and charges against. Shuttling between the Continent and Lyra's multiverse is a jolly enjoyable factor to do. The Secret Commonwealth, the second guide in Philip Pullman's Ebook of Mud collection is in shops, as is Andrzej Sapkowski's Witcher books — they weren't so simply accessible until the present got here out.
On our screens we now have Henry [ ]. This Sunday sees the start of a spectacular eight-part adaptation of Philip Pullman's His Dark Materials novels. The fantasy books, which have sold 18 million copies, are on such a vast scale. This thesis, focusing on Philip Pullman's His Dark Materials trilogy, explores the character Lyra's gender development as a result of her upbringing under parents of assorted forms and quality.
By exploring the quality of Lyra's various guardians that provide care throughout the three novels, and connecting this to. His newest book, The Secret Commonwealth, the second in a follow-up trilogy to the His Dark Materials series, The Book of Dust, appeared on October 3.
A joint HBO/BBC production of His Dark Materials will premiere in November. Pullman's legacy as a novelist seems secure, but his place as a political thinker is less established.
In honor of the upcoming Banned Books Week (September 25 to October 1), I present for your reading pleasure one of my favorite children's/young adult series, His Dark Materials by Philip Pullman.
This series bears the dubious distinction of appearing 8th on the most frequently challenged or banned books from the years to Mechanics aside, His Dark Materials is also an incredibly entertaining bit of fantasy, which explains why this series exists.
Sure, it's been more than a decade since studio execs were left scratching their heads why a blockbuster starring Nicole Kidman and Daniel Craig failed to become the next Lord of the Rings trilogy — which would have put the IP in a prime position to be rebooted.
The new series revealed one of the story's biggest twists. His Dark Materials, irrespective of its value as literature, is a story set in a Gnostic universe.
Pullman is an atheist, true, but his atheism is barely reflected in the allegory of the book. This story is far more related to Descartes' "Cogtito Ergo Sum", William Blake, and even the Matrix than the : Abigail Nussbaum.
The Golden Compass is the first installment of Pullman's His Dark Materials trilogy, three books that set out to rewrite John Milton's epic 17th century poem Paradise Lost. Milton's poem is famous for dramatizing in poetry Satan's pride, the story of humans being booted out of the Garden of Eden, notions of original sin, and loss of innocence.
His Dark Materials has been made into a BBC and HBO drama which is due to air in November His Dark Materials is followed by Pullman's The Book of Dust trilogy, which so far contains La Belle Sauvage and The Secret Commonwealth.
Over to you – what did. Philip Pullman introduced readers to his alternate Oxford, full of magic and danger, in the His Dark Materials trilogy, beginning with 's The Exclusive First Read: Philip Pullman's 'The Book Of Dust' |.
Mr Pullman's nominated book La Belle Sauvage: The Book of Dust Volume One, will return to the world of the His Dark Materials trilogy and explore concepts of free speech and address questions of Author: Alina Polianskaya.
Scholars have spent a fair amount of time exploring Philip Pullman's His Dark Materials trilogy, educating us on its weighty literary inspirations and why it is an important work of fiction.
Explaining the necessity and appeal of daemons in the trilogy (which are probably the most fascinating aspect of the books for readers) has proved a more. Following the publication of The Book of Dust: La Belle Sauvage, British author Philip Pullman is back at the forefront of the literary world, with nearly pages of gripping and undeniably rich storytelling, adding colour and depth to the universe he had created in the His Dark Materials trilogy.
The book does not pull back from showing. Philip Pullman officially launched the publication of La Belle Sauvage, the first volume in his new Book of Dust trilogy at a special event at the Bodleian Libraries this week.
La Belle Sauvage centres on the story of Malcolm, an year old boy who lives alongside the river Thames in Oxford. Exploring the origins of "His Dark Materials" back to the life of its creator, this resource also covers the creation of the trilogy, author Phillip Pullmans inspiration, response from reviewers, fans, and religious leaders, and a guide to the meaning of Pullmans alternate Guide.
[PDF Download] Philip Pullman Master Storyteller: A Guide to the Worlds of His Dark Materials. PDF Download The Science of Philip Pullmans His Dark Materials LaurelLeaf Books PDF Full Ebook.
Abachir Read Books Exploring Philip Pullman s His Dark Materials: An Unauthorized Adventure Through The Science Fiction Book: Philip. from His Dark Materials, Book Three: In a valley shaded with rhododendrons, close to the snow line, where a stream milky with meltwater splashed and where doves and linnets flew among thee immense pines, lay a cave, half-hidden by the crag above and the stiff heavy leaves that clustered below.
The woods were full. The number one New York Times best seller!. Return to the world of His Dark Materials - now an HBO original series starring Dafne Keen, Ruth Wilson, James McAvoy, and Lin-Manuel Miranda - in the second volume of Philip Pullman's new best-selling masterwork, The Book of Dust/5(K).
': Conceptualization of the Hero Within the Works of C.S. Lewis, J.R.R. Tolkien and Philip Pullman," Phil Cardew compares the heroes of The Lion, the Witch and the Wardrobe, The Return of the King, and Northern Lights (the first book in the His Dark Materials trilogy) and applies Northrop Frye's "anatomy of a hero" framework to the intellectual.This book is some ways very different in tone to His Dark Materials, or even to La Belle Sauvage., even though, through the course of those books we got a sense of a complex and developing world.
It is a distinctly Pullman voice speaking to us from the pages/5(K).
saludalmomento.club - Exploring Philip Pullmans His Dark Materials book © 2020


text:
Together alone: Sportive lemurs stay individualists in relationships
by German Primate Center
A white-footed sportive lemur in his nest. Credit: Iris Dröscher
During a one-year field study in Southern Madagascar the two researchers discovered that nocturnal white-footed sportive lemurs (Lepilemur leucopus) share a common territory with a pair partner of the opposite sex. This result clarified conflicting earlier reports on the social organization of this species. The study of the DPZ researchers also revealed a specific type of relationship model that has not yet been described for other pair-living species. Although males and females live together also outside the brief annual mating season and defend a common territory together, they were never observed to huddle or to groom each other during the more than 1,500 hours of observation. "This species is characterized by an active avoidance of pair partners," says Iris Dröscher, first author and PhD student at the Behavioral Ecology and Sociobiology Unit of the DPZ.
For their research the scientists observed a population of white-footed sportive lemurs at the Berenty Reserve and followed their movements via radio collars. They found that social interaction between couples are limited to mating once a year. "For primates, grooming is an important social interaction that strengthens the relationship between individuals. But it does not exist in white-footed sportive lemur couples," explains Iris Dröscher. "Even for sleeping, the partners choose separate trees and never spend any time together." The most elaborate social interactions of white-footed sportive lemur pair partners consist of just sitting next to each other at a small distance.
As interactions with many individuals in different contexts create cognitive challenges for animals, social complexity is regarded as an essential motor for the evolution of intelligence in primates. "White-footed sportive lemurs are characterized by a minimum of social complexity; they really define the baseline among primates", says principle investigator Peter Kappeler.
Possible explanations for why sportive lemurs are pair-living at all are currently being explored: Perhaps males can monopolize at least one female for themselves that way. Alternatively, males may stay in the vicinity of their offspring to protect them from infanticidal rivals.
Solitary lemurs avoid danger with a little help from the neighbours
Provided by German Primate Center
Citation: Together alone: Sportive lemurs stay individualists in relationships (2013, November 19) retrieved 16 July 2019 from https://phys.org/news/2013-11-sportive-lemurs-individualists-relationships.html
Social animals have more social smarts
Madagascar lemurs top endangered primates list
'Nursery nests' are better for survival of young black-and-white ruffed lemurs
DNA says lemur lookalikes are two new species
Scratching the surface of social interaction
Birds of a feather flock together to keep their options open, say scientists
New species of tree discovered in Tanzania mountains
Female mammals kill the offspring of their competitors when resources are scarce
New study on the immune system of plants: It works differently than expected


text:
\section{Introduction}

It is well known that an electric field can drive a charge current,
whereas in order to understand how to drive a spin current one
needs to resort to the field of spintronics \cite{Zutic:RoMP2004}.
Magnetization dynamics generates spin currents in adjacent normal
metal by a phenomenon known as spin pumping \cite{Berger:PRB1999,Brataas.Tserkovnyak.ea:PRB2002,Tserkovnyak.Brataas.ea:RMP2005}.
The discovery of spin pumping had a great deal of influence on the
development of the field of spintronics as it led to new insights
into the spin Hall \cite{Sinova.Valenzuela.ea:RoMP2015}, spin torque
\cite{Slonczewski:JMMM1996,Berger:PRB1996}, and spin Seebeck effects
\cite{Uchida.Xiao.ea:NM2010}. The phenomena related to the spin Seebeck
effect are studied within the field of spincaloritronics \cite{Bauer.Saitoh.ea:NM2012}
in which the focus is on interplay between the spin degrees of freedom
and heat currents.

As heat and spin currents are also carried by magnons, one naturally
arrives at a concept of magnon-mediated spin torques which can lead
to thermally induced motion of magnetic domain walls \cite{Hinzke:PRL2011,Kovalev:EPL2012,Yan.Wang.ea:PRL2011}.
Such torques exist only in noncollinear magnetic structures or when
the Dzyaloshinskii-Moriya interactions (DMI) are present. In the latter
case, such spin torques have been termed as DMI torques \cite{Manchon.Ndiaye.ea:PRB2014}.
Recently, both field-like and antidamping-like contributions to DMI
torques have been studied theoretically \cite{Linder:PRB2014,Kovalev.Guengoerdue:EEL2015,Kovalev.Zyuzin:PRB2016,Wang.Chotorlishvili.ea:PRB2016,Risinggard.Kulagina.ea:SR2016}.
It has been noted \cite{Manchon.Ndiaye.ea:PRB2014} that DMI torques
can be seen as magnon analogs of spin-orbit torques \cite{Chernyshov.Overby.ea:NP2009,Miron:Nature2010,Miron.Garello.ea:N2011,Fang.Kurebayashi.ea:NN2011,Liu:PRL2011,Liu.Pai.ea:S2012}.
This suggests that the phenomenology developed for spin-orbit torques
can be readily applied to DMI torques \cite{Freimuth.Bluegel.ea:JoPCM2014,Freimuth.Bluegel.ea:JPCM2016}.
In particular, the intrinsic contribution to DMI torques has been
identified \cite{Kovalev.Zyuzin:PRB2016}. Continuing this analogy,
one can identify fictitious electric fields acting on magnons due to time-dependent magnetization dynamics \cite{Guslienko.Aranda.ea:PRB2010,Kovalev:EPL2012,Guengoerdue.Kovalev:PRB2016}.
One can also identify the magnon-mediated equilibrium contribution to DMI. Due to such contribution the electron-mediated energy current calculated in response to magnetization dynamics
from the Kubo formalism contains an unphysical ground-state contribution
\cite{Freimuth.Bluegel.ea:JPCM2016} which needs to be subtracted.
Similar unphysical contributions have been identified for anomalous responses
induced by statistical forces \cite{Xiao.Yao.ea:PRL2006,Cooper.Halperin.ea:PRB1997,Qin.Niu.ea:PRL2011}.

There is a considerable interest in magnets on lattices with non-trivial geometry as they allow observation of Berry phase related phenomena such as the thermal Hall effect of magnons \cite{Onose.Ideue.ea:S2010,Katsura.Nagaosa.ea:PRL2010,Matsumoto.Murakami:PRL2011,Ideue.Onose.ea:PRB2012,
Zhang.Ren.ea:PRB2013,Zhang.Ren.ea:PRB2013,Shindou.Ohe.ea:PRB2013,Mook.Henk.ea:PRB2014,Mook.Henk.ea:PRB2014a,Hirschberger.Chisnell.ea:PRL2015,Lee.Han.ea:PRB2015}. Theoretically, the increased magnon damping \cite{Chernyshev.Maksimov:PRL2016}, Dirac magnons \cite{Fransson.Black-Schaffer.ea:PRB2016}, and the magnon-mediated spin Hall effect \cite{Kovalev.Zyuzin:PRB2016,Owerre:JAP2016,Kim.Ochoa.ea:PRL2016} have been predicted for kagome and honeycomb lattice ferromagnets. In addition, other manifestations of the Berry phase physics can arise in layered kagome \cite{Hirschberger.Chisnell.ea:PRL2015} and honeycomb \cite{Sivadas.Daniels.ea:PRB2015} ferromagnets as examined in this work.

In this work, we analyze magnon currents arising in response to magnetization
dynamics (see Fig.~\ref{fig:cartoon}). In the presence of a time-dependent magnetization, DMI can act as fictitious electric fields acting on magnons. As has been noted earlier in the introduction, the energy current carried by such magnons contains the
ground state contribution associated with magnon-mediated equilibrium DMI. Note that such corrections are important only in systems
with non-trivial Berry curvature of magnon bands. Here, we concentrate
on systems with non-trivial Berry curvature by considering various current responses in honeycomb and kagome lattice ferromagnets.
Our linear response calculation of heat currents agrees with the calculation
of magnon-mediated thermal torques \cite{Kovalev.Zyuzin:PRB2016},
thus confirming the Onsager reciprocity principle (see Fig.~\ref{fig:cartoon}). We also study the feasibility of experimental observation of such current responses.

The paper is organized as follows. In section II, we introduce the Hamiltonian describing magnons with multiple bands and calculate the equilibrium DMI. Next, within the same section, we describe pumping of magnons in response to magnetization dynamics and thermal torques within the linear response theory. In the final part of section II, we formulate the Onsager relations.
In section III, we apply our theory to honeycomb and kagome lattice ferromagnets. We conclude our paper in section IV. The Appendices A, B, C, and D contain very detailed derivations of our results.

\begin{figure} \centerline{\includegraphics[clip,width=1\columnwidth]{plot1}}
\protect\caption{(Color online) Two effects related by the Onsager reciprocity principle. Left: Magnetization dynamics pumps magnon current $\boldsymbol J_p$ and spin current $\boldsymbol J_s=- \hbar \boldsymbol J_p$. This process also involves heat current $\boldsymbol J_q$ carried by magnons. Right: A temperature gradient leads to a thermal torque with two components ${\cal T}_x$ and ${\cal T}_y$ acting on the uniform magnetization.  }
\label{fig:cartoon}
\end{figure}

\section{Theory of magnon pumping and DMI torques}
In this section, we develop a microscopic linear response theory of magnon pumping and nonequilibrium
magnonic torques applicable to multiple-magnonic-band
uniform ferromagnets with Dzyaloshinskii\textendash Moriya interactions. We note that in our theory magnons are treated as conserved particles. Gilbert damping $\alpha$ could broaden magnonic bands and introduce magnon non-conserving processes. In realistic situations $\alpha$ is typically small and such broadening effects can be disregarded. In what follows, to simplify formulas, we take the system volume $V=1$ and recover it in the final expressions (\ref{eq:field2}), (\ref{eq:field3}), and (\ref{eq:field2-1}).

\subsection{Preliminaries}

We consider a noninteracting boson Hamiltonian describing the magnon
fields, which could be, e.g., a result of the Holstein-Primakoff transformation:
\begin{equation}
\mathcal{H}=\int d\mathbf{r}\Psi^{\dagger}(\mathbf{r})H\Psi(\mathbf{r}),\label{eq:Ham}
\end{equation}
where $H$ is a Hermitian matrix of the size $N\times N$ and $\Psi^{\dagger}(\mathbf{r})=[a_{1}^{\dagger}(\mathbf{r}),\ldots,a_{N}^{\dagger}(\mathbf{r})]$
describes $N$ bosonic fields corresponding to the number of modes
within a unit cell (or the number of spin-wave bands). The Fourier
transformed Hamiltonian reads
\begin{equation}
\mathcal{H}=\sum_{\mathbf{k}}a_{k}^{\dagger}H(\mathbf{k})a_{k},\label{eq:Ham1}
\end{equation}
where $a_{k}^{\dagger}$ is the Fourier transformed vector of creation
operators. Hamiltonian in Eq.~(\ref{eq:Ham1}) can be diagonalized
by a unitary matrix $T_{k}$, i.e. $\mathcal{E}_{k}=T_{k}^{\dagger}H(\mathbf{k})T_{k}$
and $T_{k}^{\dagger}T_{k}=1_{N\times N}$ where $\mathcal{E}_{k}$
is the diagonal matrix of band energies, and $1_{N\times N}$ is the
$N\times N$ unit matrix.

\subsection{Magnon-mediated Dzyaloshinskii-Moriya interaction}

As magnons can exert a torque on magnetization even
in equilibrium, we begin by considering an equilibrium
state of the system. Such equilibrium DMI torques can be
captured by calculating the DMI tensor in the presence
of magnons in equilibrium state. The torque
operator is introduced as
\begin{equation}
\boldsymbol{\mathcal{T}}=\partial_{\mathbf{m}}\mathcal{H}\times\mathbf{m},\label{eq:op-torque}
\end{equation}
where $\mathbf{m}$ is a unit vector in the direction of the spin
density. We then interpret DMI in terms of the moments of the torque:
\begin{equation}
D_{\alpha\beta}=\dfrac{1}{2}\left\langle {\textstyle {\displaystyle \int}}d\mathbf{r}\Psi^{\dagger}(\mathbf{r})\left(\mathcal{T}_{\alpha}x_{\beta}+x_{\beta}\mathcal{T}_{\alpha}\right)\Psi(\mathbf{r})\right\rangle _{eq},\label{eq:DMI-tensor}
\end{equation}
where we assume a finite system. In order to represent an infinite
system, we will eliminate the position operator from the final result.
The average in Eq.~(\ref{eq:DMI-tensor}) has been calculated in Ref.
\cite{Kovalev.Zyuzin:PRB2016} in a form of a tensor $\mathbf{M}_{\beta}$
defined as
\begin{equation}
\mathbf{M}_{\beta}=\frac{1}{2}\mathrm{Tr}\left[\left(x_{\beta}\partial_{{\bf m}}H+\partial_{{\bf m}}Hx_{\beta}\right)g(\mathcal{E})\right],\label{eq:M-tensor}
\end{equation}
where $g(\mathcal{E})$ is the Bose distribution function $g(\mathcal{E})=1/[exp(\beta\mathcal{E})-1]$.
In particular, it has been found that
\begin{equation}
\mathbf{M}_{\beta}=\sum_{\mathbf{k}n}\left\{ \dfrac{1}{\beta}\ln(1-e^{-\beta\varepsilon_{nk}})B_{\mathbf{m}\beta}^{(n)}(\mathbf{k})-g(\mathcal{E}_{kn})A_{\mathbf{m}\beta}^{(n)}(\mathbf{k})\right\} ,\label{eq:Mtensor1}
\end{equation}
where (for details of this calculation see Appendix \ref{AppendixHeatDMI})
\begin{equation}
A_{\mathbf{m}\beta}^{(n)}(\mathbf{k})=\sum_{m\neq n}\mbox{Im}\left[[\widetilde{\boldsymbol{\eta}}_{k}]_{nm}\dfrac{1}{\varepsilon_{nk}-\varepsilon_{mk}}[\widetilde{v}_{k\beta}]_{mn}\right],\label{eq:A-tensor}
\end{equation}
and
\begin{equation}
B_{\mathbf{m}\beta}^{(n)}(\mathbf{k})=\sum_{m\neq n}\mbox{Im}\left[[\widetilde{\boldsymbol{\eta}}_{k}]_{nm}\dfrac{2}{(\varepsilon_{nk}-\varepsilon_{mk})^{2}}[\widetilde{v}_{k\beta}]_{mn}\right],\label{eq:B-tensor1}
\end{equation}
with the velocity $\mathbf{v}_{k}=\partial_{\mathbf{k}}H_{k}$, the
effective field $\boldsymbol{\eta}_{k}=-\partial_{{\bf m}}H_{k}$,
and their eigen basis representations, $\widetilde{\mathbf{v}}_{k}=T_{k}^{\dagger}\mathbf{v}_{k}T_{k}$
and $\widetilde{\boldsymbol{\eta}}_{k}=T_{k}^{\dagger}\boldsymbol{\eta}_{k}T_{k}$.
Finally, the expression for the DMI tensor is given by
\begin{equation}
D_{\alpha\beta}=[\mathbf{M}_{\beta}\times\mathbf{m}]_{\alpha}.\label{eq:D-tensor}
\end{equation}
It is easy to notice that $B_{\mathbf{m}\beta}^{(n)}(\mathbf{k})=-\Omega_{{\bf m}\beta}^{(n)}({\bf k})$
where now $\Omega_{{\bf m}\beta}^{(n)}({\bf k})\equiv i\left[\left(\partial_{{\bf m}}T_{{\bf k}}^{\dagger}\right)\left(\partial_{\beta}T_{{\bf k}}\right)\right]_{nn}-\left({\bf m}\leftrightarrow\beta\right)$
is the mixed space Berry curvature of the $n$th band. The second
term in Eq.~(\ref{eq:Mtensor1}) has a clear analogy to the orbital
moment \cite{Sundaram:PRB1999} which can be seen after a substitution
$\boldsymbol{\eta}_{k}\rightarrow\mathbf{v}_{k}$ \cite{Freimuth.Bluegel.ea:JoPCM2014}.

\subsection{Heat and spin pumping by magnetization dynamics}

In this subsection, we derive the magnon-mediated current response to slow magnetization dynamics in a system with broken inversion symmetry and spin-orbit interactions. The Kubo linear response energy current contains the ground state energy contribution related to the
magnon-mediated DMI which have been calculated in the previous subsection. Thus, we will use the results calculated earlier in
order to identify various transport contributions.

We are interested in the
heat, particle, and spin current density responses described by a tensor $\mathbf{t}_{a\alpha}$:
\begin{equation}
J_{a\alpha}=-\mathbf{t}_{a\alpha}\cdot\partial_{t}\mathbf{m},\label{eq:pumping}
\end{equation}
where $a$ is $q$ for the heat current, $p$ for the particle current,
and $s$ for the spin current. Here the spin current is related to
the magnon particle current density $\mathbf{J}_{p}$ by a relation $\mathbf{J}_{s}=-\hbar\mathbf{J}_{p}$.

In the presence of magnetization dynamics, Hamiltonian $\mathcal{H}$
acquires a perturbation of the form
\begin{equation}
\mathcal{H}^{'}={\textstyle {\displaystyle \int}}d\mathbf{r}\Psi^{\dagger}(\mathbf{r})H^{'}\Psi(\mathbf{r}),\label{eq:perturbation}
\end{equation}
where $H^{'}=\partial_{{\bf m}}H\cdot\delta{\bf m}(t)$ and we assume
that $\delta{\bf m}(t)$ is small. We are interested in a linear response
to the time derivative of $\mathbf{m}(t)$, thus we write $\delta{\bf m}(t)=(1/i\omega)\partial_{t}\mathbf{m}$.
Note that this calculation is similar to the calculation of dc current
response to electric field with the correspondence $\mathbf{A}(t)\rightarrow\delta{\bf m}(t)$
where the perturbation in Eq.~(\ref{eq:perturbation}) leads to an
analog of equilibrium diamagnetic current correction. Using the linear
response Kubo theory we obtain for the heat and particle current density response:
\begin{equation}
J_{a\alpha}^{K}=\bigl\langle J_{a\alpha}^{[0]}\bigr\rangle_{ne}+\bigl\langle J_{a\alpha}^{[1]}\bigr\rangle_{eq},\label{eq:field}
\end{equation}
or
\begin{equation}
J_{a\alpha}^{K}=\lim_{\omega\rightarrow0}\left\{ -\boldsymbol{\Pi}_{\alpha}^{R}(\omega)/i\omega\right\} \partial_{t}\mathbf{m}+\bigl\langle J_{a\alpha}^{[1]}\bigr\rangle_{eq},\label{eq:field1}
\end{equation}
where $\boldsymbol{\Pi}_{\alpha}^{R}(\omega)=\boldsymbol{\Pi}_{\alpha}(\omega+i0)$
is the retarded correlation function related to the following correlator
in Matsubara formalism, $\boldsymbol{\Pi}_{\alpha}(i\omega)=-\int_{0}^{\beta}d\tau e^{i\omega\tau}\bigl\langle T_{\tau}J_{a\alpha}^{[0]}\mathbf{h}\bigr\rangle$
with $\mathbf{h}=-\int d\mathbf{r}\Psi^{\dagger}(\mathbf{r})\partial_{{\bf m}}H\Psi(\mathbf{r})$
being the nonequilibrium field, and $\mathbf{j}_{q}^{[0]}(\mathbf{r})=(1/2)\Psi^{\dagger}(\mathbf{r})(\mathbf{v}H+H\mathbf{v})\Psi(\mathbf{r})$
and $\mathbf{J}_{q}^{[0]}=\int d\mathbf{r}\mathbf{j}_{q}^{[0]}(\mathbf{r})$
being the heat current density and the macroscopic heat current, respectively.
For the particle current we have similar expressions $\mathbf{j}_{p}^{[0]}(\mathbf{r})=\Psi^{\dagger}(\mathbf{r})\mathbf{v}\Psi(\mathbf{r})$
and $\mathbf{J}_{p}^{[0]}=\int d\mathbf{r}\mathbf{j}_{p}^{[0]}(\mathbf{r})$.
Here the velocity operator is given by $\mathbf{v}=(1/i\hbar)[\mathbf{r},H]$.
We also introduce a gradient correction to the heat and particle currents
due to perturbation, i.e., $\mathbf{J}_{a}^{[1]}=\int d\mathbf{r}\mathbf{j}_{a}^{[1]}(\mathbf{r})$
where $\mathbf{j}_{q}^{[1]}(\mathbf{r})=(1/2)\Psi^{\dagger}(\mathbf{r})[(\delta{\bf m}(t)\cdot\partial_{{\bf m}})(\mathbf{v}H+H\mathbf{v})]\Psi(\mathbf{r})$
and $\mathbf{j}_{s}^{[1]}(\mathbf{r})=\Psi^{\dagger}(\mathbf{r})[\delta{\bf m}(t)\cdot\partial_{{\bf m}}\mathbf{v}]\Psi(\mathbf{r})$.
This analog of diamagnetic current cancels with the term $\boldsymbol{\Pi}_{\alpha}^{R}(0)$
resulting in the Kubo contribution of the form
\begin{equation}
J_{a\alpha}^{K}=\lim_{\omega\rightarrow0}\left\{ [\boldsymbol{\Pi}_{\alpha}^{R}(0)-\boldsymbol{\Pi}_{\alpha}^{R}(\omega)]/i\omega\right\} \partial_{t}\mathbf{m}.\label{eq:Kubo}
\end{equation}
The correlation function in Eq.~($\ref{eq:Kubo}$) is calculated by
considering the simplest bubble diagram for $\boldsymbol{\Pi}_{\alpha}$
and performing the analytic continuation, see e.g. Ref. \cite{Kovalev.Zyuzin:PRB2016}.
We express the result through a response tensor $\mathbf{t}_{a\alpha}^{K}$
containing two contributions $\mathbf{t}_{a\alpha}^{K}=\mathbf{t}_{a\alpha}^{\text{I}}+\mathbf{t}_{a\alpha}^{\text{II}}$,
which are given by
\begin{equation}
\begin{array}{c}
\mathbf{t}_{a\alpha}^{\text{I}}=\dfrac{1}{\hbar}{\displaystyle \int}\dfrac{d\omega}{2\pi}g(\omega)\dfrac{d}{d\omega}\mbox{Re}\mbox{Tr}\bigl\langle\mathcal{J}_{a\alpha}G^{R}\boldsymbol{\eta}G^{A}-\mathcal{J}_{a\alpha}G^{R}\boldsymbol{\eta}G^{R}\bigr\rangle,\\
\mathbf{t}_{a\alpha}^{\text{II}}=\dfrac{1}{\hbar}{\displaystyle \int}\dfrac{d\omega}{2\pi}g(\omega)\mbox{Re}\mbox{Tr}\bigl\langle\mathcal{J}_{a\alpha}G^{R}\boldsymbol{\eta}\dfrac{dG^{R}}{d\omega}-\mathcal{J}_{a\alpha}\dfrac{dG^{R}}{d\omega}\boldsymbol{\eta}G^{R}\bigr\rangle,
\end{array}\label{eq:t-tensor}
\end{equation}
where $g(\omega)$ is the Bose distribution function $g(\omega)=1/[\exp(\hbar\omega/k_{B}T)-1]$,
$G^{R}=\hbar(\hbar\omega-H+i\Gamma)^{-1}$, $G^{A}=\hbar(\hbar\omega-H-i\Gamma)^{-1}$,
$\boldsymbol{\eta}=-\partial_{{\bf m}}H$ , $\boldsymbol{\mathcal{J}}_{q}=(\mathbf{v}H+H\mathbf{v})/2$,
and $\boldsymbol{\mathcal{J}}_{p}=\mathbf{v}$. In our calculations,
we adopt a phenomenological treatment and relate the quasiparticle
broadening to the Gilbert damping, i.e. $\Gamma=\alpha\hbar\omega$.

Note that the Kubo response for the energy current density in Eq.~(\ref{eq:Kubo})
contains the bound energy current associated with DMI:
\begin{equation}
\mathbf{J}_{q}^{D}=\hat{D}\cdot(\mathbf{m}\times\partial_{t}\mathbf{m}),\label{eq:DMIsubtraction}
\end{equation}
where tensor $\hat{D}$ is given in Eq.~(\ref{eq:D-tensor}). This
current needs to be subtracted from the Kubo current in Eq.~(\ref{eq:Kubo})
in order to obtain a transport heat current:
\begin{equation}
\mathbf{J}_{q\alpha}=\mathbf{J}_{q\alpha}^{K}-\mathbf{J}_{q}^{D}.\label{eq:subtraction}
\end{equation}
To express the response tensor $\mathbf{t}_{a\alpha}^{K}$, we use
the Fourier transformed operators and the eigen basis representation
for the velocity, $\hbar\widetilde{\mathbf{v}}_{k}=\partial_{\mathbf{k}}\mathcal{E}_{k}-i\boldsymbol{\mathcal{A}}_{k}\mathcal{E}_{k}+i\mathcal{E}_{k}\boldsymbol{\mathcal{A}}_{k}$,
and the effective field, $-\widetilde{\boldsymbol{\eta}}_{k}=\partial_{\mathbf{m}}\mathcal{E}_{k}-i\boldsymbol{\mathcal{A}}_{m}\mathcal{E}_{k}+i\mathcal{E}_{k}\boldsymbol{\mathcal{A}}_{m}$,
where $\boldsymbol{\mathcal{A}}_{k}=iT_{k}^{\dagger}\partial_{\mathbf{k}}T_{k}$
and $\boldsymbol{\mathcal{A}}_{m}=iT_{k}^{\dagger}\partial_{\mathbf{m}}T_{k}$.
For the details of derivation of intrinsic contribution to the heat current see Appendix \ref{AppendixHeat}.
We obtain
\begin{equation}
\begin{array}{c}
\mathbf{t}_{q\alpha}^{K}={\displaystyle \sum_{\mathbf{k}n}}\Bigl\{ g(\varepsilon_{nk})[-\varepsilon_{nk}B_{\mathbf{m}\alpha}^{(n)}(\mathbf{k})+A_{\mathbf{m}\alpha}^{(n)}(\mathbf{k})]\\
-\dfrac{\varepsilon_{nk}g'(\varepsilon_{nk})}{2\Gamma^{(n)}_{k}}(\partial_{\mathbf{m}}\varepsilon_{nk})(\partial_{k_{\alpha}}\varepsilon_{nk})\Bigr\},
\end{array}\label{eq:t-tensor2}
\end{equation}
which after combining with DMI energy current $\mathbf{J}_{q}^{D}$
leads to the response tensor describing the heat current (see Appendix \ref{AppendixHeatOverall}):

\begin{equation}
\begin{array}{c}
\mathbf{t}_{q\alpha}^{ex}=-\dfrac{1}{V}{\displaystyle \sum_{\mathbf{k}}{\displaystyle \sum_{n=1}^{N}}\dfrac{1}{2\Gamma^{(n)}_{k}}(\partial_{{\bf m}}\varepsilon_{nk})(\partial_{k_{\alpha}}\varepsilon_{nk})\varepsilon_{nk}g'(\varepsilon_{nk})},\\
\mathbf{t}_{q\alpha}^{in}=\dfrac{1}{V}{\displaystyle \sum_{\mathbf{k}}}{\displaystyle \sum_{n=1}^{N}}c_{1}(\varepsilon_{nk})\Omega_{{\bf m}k_{\alpha}}^{(n)}(\mathbf{k}),
\end{array}\label{eq:field2}
\end{equation}
where \textbf{$\varepsilon_{nk}=[\mathcal{E}_{k}]_{nn}$}, $\Gamma^{(n)}_{k}=\alpha\varepsilon_{nk}$,
$g'(\varepsilon_{nk})=(2k_{B}T)^{-1}\{1-\cosh(\varepsilon_{nk}/k_{B}T)\}^{-1}$,
$c_{1}[\varepsilon_{nk}]=g(\varepsilon_{nk})\varepsilon_{nk}-(1/\beta)\ln(1-e^{-\beta\varepsilon_{nk}})$,
$V$ is volume, and we separated the total tensor $\mathbf{t}_{q\alpha}$
into the intrinsic and extrinsic contributions, i.e., $\mathbf{t}_{q\alpha}=\mathbf{t}_{q\alpha}^{ex}+\mathbf{t}_{q\alpha}^{in}$.
For the particle current response only $\mathbf{t}_{p\alpha}^{K}$
tensor needs to be considered, thus we obtain the following expression
for the total tensor, $\mathbf{t}_{p\alpha}=\mathbf{t}_{p\alpha}^{ex}+\mathbf{t}_{p\alpha}^{in}$,
divided into the intrinsic and extrinsic contributions (for details of calculations of intrinsic contribution see Appendix \ref{AppendixCurrent}):
\begin{equation}
\begin{array}{c}
\mathbf{t}_{p\alpha}^{ex}=-\dfrac{1}{V}{\displaystyle \sum_{\mathbf{k}}{\displaystyle \sum_{n=1}^{N}}\dfrac{1}{2\Gamma^{(n)}_{k}}(\partial_{{\bf m}}\varepsilon_{nk})(\partial_{k_{\alpha}}\varepsilon_{nk})g'(\varepsilon_{nk})},\\
\mathbf{t}_{p\alpha}^{in}=\dfrac{1}{V}{\displaystyle \sum_{\mathbf{k}}}{\displaystyle \sum_{n=1}^{N}}g(\varepsilon_{nk})\Omega_{{\bf m}k_{\alpha}}^{(n)}(\mathbf{k}).
\end{array}\label{eq:field3}
\end{equation}
The last tensor also describes the spin current response, i.e., $\mathbf{t}_{s\alpha}=-\hbar\mathbf{t}_{p\alpha}$.

\subsection{Thermal torques}

In this subsection, we derive the magnon-mediated magnetization torque
response to a temperature gradient in a system with broken inversion
symmetry and spin-orbit interactions. For details of derivations see Appendix \ref{AppendixTorque}.
The thermal torque is defined
according to equation
\begin{equation}
\boldsymbol{\mathcal{T}}=-\boldsymbol{\beta}_{\alpha}\partial_{\alpha}T,
\end{equation}
where $\boldsymbol{\beta}_{\alpha}$ is the thermal torkance tensor
and $\boldsymbol{\mathcal{T}}$ describes torque acting on magnetization
and leading to modification of the Landau-Lifshitz-Gilbert equation,
i.e., $s(1+\alpha\mathbf{m}\times)\dot{\mathbf{m}}=\mathbf{m}\times\mathbf{H}_{\text{eff}}+\boldsymbol{\mathcal{T}}$
where $\mathbf{H}_{\text{eff}}$ is the effective magnetic field and
$s$ is the spin density. We use the Luttinger linear response method
\cite{Luttinger:PR1964} in which the temperature gradient is replicated
by a perturbation to Hamiltonian $\mathcal{H}$ of the form
\begin{equation}
\mathcal{H}^{'}=\dfrac{1}{2}\int d\mathbf{r}\Psi^{\dagger}(\mathbf{r})\left(H\chi+\chi H\right)\Psi(\mathbf{r}),\label{eq:Luttinger}
\end{equation}
where we introduce the temperature gradient as $\partial_{i}\chi=-\partial_{i}T/T$.
The torque response can be found by calculating the effective magnon-mediated
field:
\begin{equation}
\mathbf{h}=\mathbf{h}^{[0]}+\mathbf{h}^{[1]}=-\bigl\langle\partial_{\mathbf{m}}\mathcal{H}\bigr\rangle_{ne}-\bigl\langle\partial_{\mathbf{m}}\mathcal{H}^{'}\bigr\rangle_{eq},\label{eq:Tfield}
\end{equation}
where for the second term the averaging is done over the equilibrium
state and for the first term over nonequilibrium state induced by
the temperature gradient. The magnon-mediated torque acting on the
magnetization is given by
\begin{equation}
\boldsymbol{\mathcal{T}}=\mathbf{m}\times\mathbf{h}.\label{eq:torque}
\end{equation}
Within the linear response theory, the response $\mathbf{h}^{[0]}$
to a temperature gradient can be calculated from expression
\begin{equation}
\mathbf{h}^{[0]}=\lim_{\Omega\rightarrow0}\left\{ [\boldsymbol{\Pi}_{\alpha}^{R}(\Omega)-\boldsymbol{\Pi}_{\alpha}^{R}(0)]/i\Omega\right\} \partial_{\alpha}\chi,\label{eq:Tfield1}
\end{equation}
where $\boldsymbol{\Pi}_{\alpha}^{R}(\Omega)=\boldsymbol{\Pi}_{\alpha}(\Omega+i0)$
is the retarded correlation function related to the following correlator
in Matsubara formalism, $\boldsymbol{\Pi}_{\alpha}(i\Omega)=-\int_{0}^{\beta}d\tau e^{i\Omega\tau}\bigl\langle T_{\tau}\mathbf{h}J_{q\alpha}^{[0]}\bigr\rangle$.
Note that this correlator differs from the one arising in Eq.~(\ref{eq:field1})
in the order of operators. In the correlator, we reduce the perturbation
$\mathcal{H}^{'}$ to the energy current by employing the equality
$\mathcal{\dot{H}}^{'}=(i/\hbar)[\mathcal{H},\mathcal{H}^{'}]=\mathbf{J}_{q}^{[0]}\boldsymbol{\partial}\chi$
and integration by parts. Following the notations in Ref. \cite{Kovalev.Zyuzin:PRB2016},
we introduce the linear response tensors $\mathbf{S}_{\alpha}$ and
$\mathbf{M}_{\alpha}$ for the fields $\mathbf{h}^{[0]}$ and $\mathbf{h}^{[1]}$
and the total response tensor $\mathbf{L}_{\alpha}=\mathbf{S}_{\alpha}+\mathbf{M}_{\alpha}$
according to equation
\begin{equation}
\mathbf{h}^{[0]}+\mathbf{h}^{[1]}=-\mathbf{L}_{\alpha}\partial_{\alpha}\chi,\label{eq:eff-field}
\end{equation}
where $\mathbf{M}_{\alpha}$ is given by Eq.~(\ref{eq:M-tensor})
as it follows from Eq.~(\ref{eq:Tfield}). For the tensors $\mathbf{S}_{\alpha}$
we obtain
\begin{equation}
\begin{array}{c}
\mathbf{S}_{\alpha}={\displaystyle \sum_{\mathbf{k}n}}\Bigl\{ g(\varepsilon_{nk})[-\varepsilon_{nk}B_{\mathbf{m}\beta}^{(n)}(\mathbf{k})+A_{\mathbf{m}\beta}^{(n)}(\mathbf{k})]\\
+\dfrac{\varepsilon_{nk}g'(\varepsilon_{nk})}{2\Gamma^{(n)}_{k}}(\partial_{\mathbf{m}}\varepsilon_{nk})(\partial_{k_{\beta}}\varepsilon_{nk})\Bigr\}.
\end{array}\label{eq:S-tensor}
\end{equation}
We can also separate the total response tensor into the intrinsic
and extrinsic contributions:
\begin{equation}
\begin{array}{c}
\mathbf{L}_{\alpha}^{ex}=\dfrac{1}{V}{\displaystyle \sum_{\mathbf{k}}{\displaystyle \sum_{n=1}^{N}}\dfrac{1}{2\Gamma^{(n)}_{k}}(\partial_{{\bf m}}\varepsilon_{nk})(\partial_{k_{\alpha}}\varepsilon_{nk})\varepsilon_{nk}g'(\varepsilon_{nk})},\\
\mathbf{L}_{\alpha}^{in}=\dfrac{1}{V}{\displaystyle \sum_{\mathbf{k}}}{\displaystyle \sum_{n=1}^{N}}c_{1}(\varepsilon_{nk})\Omega_{{\bf m}k_{\alpha}}^{(n)}(\mathbf{k}).
\end{array}\label{eq:field2-1}
\end{equation}
 For the thermal torkance tensor, we obtain
\begin{equation}
\boldsymbol{\beta}_{\alpha}=\mathbf{L}_{\alpha}\times\mathbf{m}/T.\label{eq:torkance}
\end{equation}

\subsection{Onsager reciprocity relation}

We are now in the position to combine the results from previous subsections
into one expression that emphasized the Onsager reciprocity relation.
In principle, the result of calculation of thermal torques in the
last section can be extracted from the Onsager relations without performing
the calculation. Writing the response tensors in terms of the torkance
tensors, we obtain
\begin{equation}
\begin{array}{l}
\left(\begin{array}{c}
J_{p\alpha}\\
J_{q\alpha}\\
\boldsymbol{\mathcal{T}}
\end{array}\right)=\\
\\
\qquad\left(\begin{array}{ccc}
\hat{\sigma}(\mathbf{m}) & \hat{\Pi}^{T}(-\mathbf{m}) & \boldsymbol{\alpha}_{\alpha}(-\mathbf{m})\\
\hat{\Pi}(\mathbf{m}) & T\hat{\lambda}(\mathbf{m}) & T\boldsymbol{\beta}_{\alpha}(-\mathbf{m})\\
\boldsymbol{\alpha}_{\alpha}(\mathbf{m}) & T\boldsymbol{\beta}_{\alpha}(\mathbf{m}) & -\hat{\varLambda}(\mathbf{m})
\end{array}\right)\left(\begin{array}{c}
-\partial_{\alpha}\varphi\\
\partial_{\alpha}\chi\\
\mathbf{m}\times\partial_{t}\mathbf{m}
\end{array}\right),
\end{array}\label{eq:Onsager}
\end{equation}
where summation over repeated indices is implied, and we introduced
the conductivity tensor $\hat{\sigma}(\mathbf{m})$, the magnonic heat
conductivity
tensor $\hat{\lambda}(\mathbf{m})$, the tensor $\hat{\Pi}(\mathbf{m})$
describing the magnon Seebeck and Peltier effects, and the tensor
$\hat{\varLambda}(\mathbf{m})$ corresponding to LLG equation. The
tensor $\boldsymbol{\alpha}_{\alpha}(\mathbf{m})$ was introduced
by analogy with the tensor $\boldsymbol{\beta}_{\alpha}(\mathbf{m})$
and it is given in Eq.~(\ref{eq:field3}), i.e., $\boldsymbol{\alpha}_{\alpha}(-\mathbf{m})=\mathbf{t}_{p\alpha}\times\mathbf{m}$.
For completeness we also added a response to an analog of electric
field for magnons, $-\partial_{\alpha}\varphi$ \cite{Cornelissen.Peters.ea:PRB2016}. Equation (\ref{eq:Onsager})
immediately follows from Eqs. (\ref{eq:field2}), (\ref{eq:field3}),
and (\ref{eq:field2-1}) given that intrinsic contributions are odd
and extrinsic contributions are even under magnetization reversal.
The Onsager reciprocity relation in Eq.~(\ref{eq:Onsager}) is similar
to expressions obtained for similar electron-mediated effects in Ref.~\cite{Freimuth.Bluegel.ea:JoPCM2014}. Equation (\ref{eq:Onsager})
can be modified to account for the possibility of magnon accumulation
resulting from the magnon motive force \cite{Guengoerdue.Kovalev:PRB2016}
or temperature gradient \cite{Cornelissen.Peters.ea:PRB2016}.

\section{Results for honeycomb and kagome ferromagnets}
In this section, we apply our theory to single layer honeycomb and kagome ferromagnets with DMI.
In our models, we introduce two types of DMI. The Rashba DMI correspond to mirror asymmetry in the system (see Figs.~\ref{fig:graphene} and \ref{fig:kagome}). The remaining DMI make the second quantized Hamiltonian of magnons to be asymmetric under time reversal. Such asymmetries make our systems to exhibit behavior analogous to electronic systems lacking the center of inversion and time reversal symmetry \cite{Freimuth.Bluegel.ea:JPCM2016}.
To demonstrate explicitly how fictitious electric fields result in magnon currents, we describe the honeycomb system analytically. Our results could also be relevant to three-dimensional layered structures with weakly coupled layers.
Note that the magnon pumping could in principle be modified by DMI induced anharmonic interactions of magnons \cite{Chernyshev.Maksimov:PRL2016}. We do not expect this effect to be large when magnetization substantially deviates from the direction orthogonal to DMI vector.

\subsection{Application to honeycomb ferromagnet}
\begin{figure} \centerline{\includegraphics[clip,width=0.5\columnwidth]{graphene_soc}}

\protect\caption{Schematics of the graphene layer parameters for the tight-binding model. Vectors connecting nearest neighbors are  ${\boldsymbol \tau}_{1} = \frac{1}{2}(\frac{1}{\sqrt{3}},1 )$,
 ${\boldsymbol \tau}_{2} = \frac{1}{2}(\frac{1}{\sqrt{3}},-1)$, and ${\boldsymbol \tau}_{3} = \frac{1}{\sqrt{3}}(-1,0 )$ are used in deriving the Hamiltonian for magnons. Vectors ${\bf a}_{1} = \frac{1}{2}(\sqrt{3},1)$, and ${\bf a}_{2} = \frac{1}{2}(\sqrt{3}, -1)$ are used in deriving the second-nearest neighbor DMI.}
\label{fig:graphene}

\end{figure}
In this subsection, we study a model of an insulating ferromagnet on a honeycomb lattice. This model contains physics discussed above in a transparent and analytical way.  For the details of further derivations see Appendix \ref{AppendixHoneycomb}. We assume a Heisenberg exchange of ferromagnetic sign, in-plane DMI of Rashba type, and second-nearest neighbor DMI.
The Hamiltonian is
\begin{align}
H =- J\sum_{<ij>}{\bf S}_{i}{\bf S}_{j}
&+ \sum_{<ij>} {\bf D}^{[\mathrm{R}]}\left[ {\bf S}_{i}\times {\bf S}_{j} \right]
\\
&
+ D^{[\mathrm{z}]}\sum_{<<ij>>}\nu_{ij} \left[ {\bf S}_{i}\times {\bf S}_{j} \right]_{z}.
\end{align}
The vectors of the Rashba type DMI are shown in Fig.~\ref{fig:graphene}, where ${\bf d}_{1} = \frac{1}{2}(\sqrt{3},-1)$, ${\bf d}_{2} = \frac{1}{2}(-\sqrt{3},-1)$, and ${\bf d}_{3} = (0,1)$, such as ${\bf D}^{[\mathrm{R}]} = D^{[\mathrm{R}]}{\bf d}$. Note that all vectors, such as $\boldsymbol\tau_i$ and $\boldsymbol a_i$, are measured in units of lattice spacing $\text{a}_0$ which is recovered in the final result. The vector of the second-nearest neighbor DMI is in the $z-$ direction, and the signs of $\nu_{ij}$ are depicted in green in Fig.~\ref{fig:graphene} for the directions shown by dashed green arrows. For analytical results, we assume that all DMI are small, i.e. $J \gg D^{[\mathrm{R}]}$ and $J \gg  D^{[\mathrm{z}]}$.
In our model, initially, we assume that the order is in general $(m_{x}, m_{y}, m_{z})$ direction, which can be realized by application of the magnetic field. Our strategy would be to first understand the role of the DMI in the behavior of magnons for a general direction of the ferromagnetic order. After that we will assume that the main order is in the $z-$ direction, while the perturbations that deviate the order are in the $x-y$ plane (see Fig.~\ref{fig:cartoon}).
To study the magnons, we perform the Holstein-Primakoff transformation. The unit cell of the honeycomb ferromagnet has two spins ${\bf S}_{\mathrm{A}}$ and ${\bf S}_{\mathrm{B}}$, hence the two sets of boson operators, $a^{\dag}({\bf r}),~a({\bf r})$ and $b^{\dag}({\bf r}),~b({\bf r})$ corresponding to the $\mathrm{A}$ and ${\mathrm B}$ sublattices are introduced. The Holstein-Primakoff transformation reads as usual, $S^{z}_{\mathrm{A}} = S - a^{\dag}a$, and $S^{+}_{\mathrm{A}} = (S^{x}_{\mathrm{A}} + iS^{y}_{\mathrm{A}}) = \sqrt{2S-a^{\dag}a} a$ ($S$ is the total spin), and the same for $\mathrm{B}$ spins. The Fourier image of the Hamiltonian describing non-interacting magnons written in terms of the $\Psi = (a_{\bf k},~b_{\bf k})^{\mathrm{T}}$ spinor is
\begin{align}
H =JS\left[ \begin{array} {cc}
3 + \Delta_{\bf k} & -{\tilde \gamma}_{\bf k} \\
-{\tilde \gamma}^{*}_{\bf k} & 3 - \Delta_{\bf k}
\end{array} \right],
\end{align}
where $\Delta_{\bf k} = 2\Delta \left[ \sin(k_{y}) - 2\sin\left( \frac{k_{y}}{2}\right)\cos\left( \frac{\sqrt{3}k_{x}}{2} \right)  \right]$, with $\Delta =m_{z} D^{[\mathrm{z}]}/J$. This type of DMI is a ${\bf k}-$ dependent mass of magnons.  Deriving ${\tilde \gamma}_{\bf k}$ we considered Rashba DMI in the lowest order in $D^{[\mathrm{R}]}/J \ll 1$ parameter. With this assumption
\begin{align}
{\tilde \gamma}_{\bf k} = 2e^{i\frac{{\tilde k}_{x}}{2\sqrt{3}}}\cos\left(\frac{{\tilde k}_{y}}{2} \right) + e^{-i\frac{{\tilde k}_{x}}{\sqrt{3}}},
\end{align}
where ${\tilde k}_{x}  = k_{x} - \sqrt{3}\frac{D^{[\mathrm{R}]}}{J} m_{y}$, and ${\tilde k}_{y}  = k_{y} + \sqrt{3}\frac{D^{[\mathrm{R}]}}{J}m_{x}$. We observe that Rashba DMI plays an effective role of magnon charge, while order direction $(m_{x},m_{y},0)$ is an effective vector potential felt by magnons.

The eigenvalues of the Hamiltonian are calculated to be,
\begin{align}
\epsilon_{\bf k,\pm} = JS\left(3 \pm \sqrt{\Delta_{\bf k}^2 + \vert {\tilde \gamma}_{\bf k} \vert^2} \right),
\end{align}
with corresponding eigenfunctions
\begin{equation}v_{\bf k,+} = [
 \cos({\tilde \xi}_{\bf k}/2)e^{i{\tilde \chi}_{\bf k}},  ~
 -\sin({\tilde \xi}_{\bf k}/2)  ]^{T},\end{equation}
and
\begin{equation}v_{\bf k,-} = [
 \sin({\tilde \xi}_{\bf k}/2) ,~
 \cos({\tilde \xi}_{\bf k}/2) e^{-i{\tilde \chi}_{\bf k}}
]^{T},\end{equation}
where $\sin({\tilde \xi}_{\bf k}) =  \vert {\tilde \gamma}_{\bf k}\vert/\sqrt{\Delta_{\bf k}^2 + \vert {\tilde \gamma}_{\bf k} \vert^2}$, and ${\tilde \gamma}_{\bf k} = \vert{\tilde \gamma}_{\bf k}\vert e^{i{\tilde \chi}_{\bf k}}$, and the tilde symbol here means that corresponding ${\bf k}$ momenta are shifted by the Rashba DMI. Unitary matrix that diagonalizes the Hamiltonian is readily constructed and it is given by
\begin{align}
T_{\bf k} = \left[ \begin{array}{cc}
 \cos\left(\frac{{\tilde \xi}_{\bf k}}{2}\right)e^{i{\tilde \chi}_{\bf k}} &  \sin\left(\frac{{\tilde \xi}_{\bf k}}{2}\right) \\
- \sin\left(\frac{{\tilde \xi}_{\bf k}}{2}\right)  & \cos\left(\frac{{\tilde \xi}_{\bf k}}{2}\right) e^{-i{\tilde \chi}_{\bf k}}
\end{array}\right].
\end{align}
We are now ready to derive spin and heat currents which are driven by magnetization dynamics.
We set the dominant component of the ferromagnetic order in the $z-$ direction and assume that the magnetization dynamics is in the $x-y$ plane. We only focus on the intrinsic contribution to the currents, i.e., due to non-trivial Berry curvatures of the magnon band structure.
An expression defining the Berry curvature is
\begin{align}
&\Omega_{\alpha, m_{\beta}}=2\mathrm{Im}\left[ \left( \partial_{\alpha}T_{\bf k}^{\dag}\right)\left( \partial_{m_{\beta}}T_{\bf k}\right) \right]
= \frac{1}{2}\sin\left({\tilde \xi}_{\bf k} \right)
\\
& \times \left[ \left( \partial_{\alpha}{\tilde \chi}_{\bf k}\right) \left(\partial_{m_{\beta}}{\tilde \xi}_{\bf k}\right) - \left(\partial_{m_{\beta}}{\tilde \chi}_{\bf k}\right) \left(\partial_{\alpha}{\tilde \xi}_{\bf k}\right) \right]
\left[\begin{array} {cc}
1 & 0 \\
0 & - 1
\end{array}
\right].
\end{align}
In the following, we focus on the $\alpha = x$ and $\beta = x$ case, and mention $\beta = y$ case at the end.
Recall that $\Delta_{\bf k}$ does not depend on $m_{\beta}$ for $\beta =(x,y)$ components, hence $\partial_{m_\beta}\Delta_{\bf k} = 0$.
The derivative with respect to the direction of the order $m_{\beta}$ of the remaining functions that depend on ${\tilde {\bf k}}$ is
\begin{align}
&
\frac{\partial}{\partial m_{x}} = \sqrt{3}\frac{D^{[\mathrm{R}]}}{J} \frac{\partial}{\partial {\tilde k}_{y}}
\equiv \sqrt{3}\frac{D^{[\mathrm{R}]}}{J}\partial_{y},
\\
&
\frac{\partial}{\partial m_{y}} = -\sqrt{3}\frac{D^{[\mathrm{R}]}}{J} \frac{\partial}{\partial {\tilde k}_{x}}
\equiv - \sqrt{3}\frac{D^{[\mathrm{R}]}}{J}\partial_{x}.
\end{align}
This straightforward transformation makes the mixed Berry curvature a regular ${\bf k}-$ space one, except for the $\partial_{m_\beta}\Delta_{\bf k} = 0$ condition. The Berry curvature has extrema at the ${\bf K}^\prime = \left(0, \frac{4\pi}{3} \right)$ and ${\bf K} = \left(0, -\frac{4\pi}{3} \right)$ points, and can be approximated as
\begin{align}
\Omega_{x, m_{x}}\vert_{{\bf K}({\bf K}^\prime)} \approx - \frac{27}{8}\frac{D^{[\mathrm{R}]}}{J} \frac{\Delta}{ \left( 27\Delta^2 + \frac{3}{4}k^2 \right)^{3/2}}
\left[\begin{array} {cc}
1 & 0 \\
0 & - 1
\end{array}\right].
\end{align}
The curvature is the same for both ${\bf K}^\prime$ and ${\bf K}$ points. The spectrum at these points is finite, $\epsilon_{\bf k,\pm} \approx JS(3 \pm 3\sqrt{3} \vert\Delta\vert)$, but the Berry curvature is of the monopole type.
Hence at small temperatures, despite the exponential suppression of the magnon number at the ${\bf K}^\prime$ and ${\bf K}$ points, there might be a contribution to the magnon currents due to this Berry curvature.
At the ${\bf \Gamma} =(0,0)$ the spectrum of the lowest band is $\epsilon_{\bf k, -} \approx \frac{1}{4}SJk^2$, and it will be populated by the magnons the most at low temperatures. The Berry curvature is approximated close to this point as
\begin{align}
\Omega_{x, m_{x}}\vert_{{\bf \Gamma}} \approx  - \frac{D^{[\mathrm{R}]}}{J} \frac{\Delta}{48} k_{y}^2 k_{x}^2 \left[\begin{array} {cc}
1 & 0 \\
0 & - 1
\end{array}\right].
\end{align}
According to Eqs.~(\ref{eq:pumping}) and (\ref{eq:field3}), the particle current density due to the Berry curvature at small temperatures, $SJ \gg T$, reads
\begin{align}\label{spin_honeycomb}
J_{px}
=  \frac{ D^{[\mathrm{R}]}}{J} \frac{\sqrt{3}}{\text{a}_0\pi}
&\bigg[  \sinh\left[ \frac{1}{z} \frac{3\sqrt{3}D^{[\mathrm{z}]}}{J}\right] e^{-\frac{3}{z}}
\\
&
+ \frac{D^{[\mathrm{z}]}}{J} \frac{\sqrt{3} \zeta(3) }{36} z^3 \bigg] \left( \partial_{t}{\bf m}\right)_{x},
\nonumber
\end{align}
where we introduced $ z = T/SJ$ for brevity, and set $m_{z} = 1$.
Similarly, from Eq.~(\ref{eq:t-tensor2}), the heat current due to the Berry curvature at  small temperatures, $SJ \gg T$, reads
\begin{align}\label{heat_honeycomb}
J_{qx} =
JS \frac{D^{[\mathrm{R}]}}{J}\frac{3\sqrt{3}}{\text{a}_0\pi}
&
\bigg[  \sinh\left( \frac{1}{z} \frac{3\sqrt{3}D^{[\mathrm{z}]}}{J}\right) e^{-\frac{3}{z}}
\\
&
+ \frac{D^{[\mathrm{z}]}}{J} \frac{\sqrt{3}I}{216}z^4
\bigg]\left( \partial_{t}{\bf m}\right)_{x}.
\nonumber
\end{align}
In both cases a term $\propto e^{-\frac{3SJ}{T}}$ is due to ${\bf K}^\prime$ and ${\bf K}$ points, while the remaining one is due to ${\bf \Gamma}$ point. We introduced a numerical constant $I = \int_{0}^{\infty}dx x^2 \left[ x\frac{e^x}{e^x-1} - \ln(e^x - 1) \right]=4\pi^4/45 \approx 8.65$, and Riemann zeta-function $\zeta(3)\approx 1.2$.

\begin{figure} \centerline{\includegraphics[clip, width=1\columnwidth]{vlad}}

\protect\caption{(Color online) Left: The even component under magnetization reversal of the tensor $\alpha_{ij}$ as a function of temperature. Right:  The even component under magnetization reversal of the torkance tensor $\beta_{ij}$ as a function of temperature. In both cases the magnetization is along the $z-$ axis. For the strength of DMI we use $D^{[z]}=D^{[R]}=J/6$. Red curves correspond to numerical results and blue curves correspond to analytical results in Eqs.~(\ref{spin_honeycomb}) and (\ref{heat_honeycomb}).  }

\label{fig:spinheat}

\end{figure}

It is straightforward to show that Berry curvature parts of the $J_{px}$ and $J_{qx}$ currents driven by $\left(\partial_{t} {\bf m}\right)_{y}$ magnetization dynamics vanish. The $J_{sy}$ and $J_{qy}$ currents driven by $\left(\partial_{t} {\bf m}\right)_{y}$ magnetization dynamics will have the same expressions as in Eqs.~(\ref{spin_honeycomb}) and (\ref{heat_honeycomb}). Thus, we calculated even under magnetization reversal components $\alpha_{xy}^\text{even}=-\alpha_{yx}^\text{even}$ and $\beta_{xy}^\text{even}=-\beta_{yx}^\text{even}$ as it follows from Eq.~(\ref{eq:Onsager}). As can be seen from Fig.~\ref{fig:spinheat}, Eqs.~(\ref{spin_honeycomb}) and (\ref{heat_honeycomb}) only qualitatively agree with the numerical results at higher temperatures as the Berry curvature from other parts of the Brillouin zone starts to contribute to the result.

\subsection{Application to kagome ferromagnet}

Here we apply our theory to the kagome lattice ferromagnet with the nearest neighbor DMI. The lattice of the system and its magnon
spectrum are shown in Fig.~\ref{fig:kagome}. Note that all vectors, such ${\bf a}_1$ and ${\bf a}_2$, are measured in units of lattice spacing $\text{a}_0$ which is recovered in the final result. We consider a model
considered in Ref. \cite{Kovalev.Zyuzin:PRB2016} with a Hamiltonian given by
\begin{align}
H=-J\sum_{<ij>}{\bf S}_{i}{\bf S}_{j}-B\sum_{i}S_{i}^{z}+\sum_{<ij>}\nu_{ij}\mathbf{D}_{ij}\left[{\bf S}_{i}\times{\bf S}_{j}\right],\label{eq:Ham}
\end{align}
where $J>0$ corresponds to ferromagnetic nearest neighbor exchange,
$B$ is the external magnetic field, and $\nu_{ij}$ describes a sign
convention for the nearest neighbor DMI, i.e., $\nu_{ij}=1$ for the
clockwise sense of direction and $\nu_{ij}=-1$ otherwise (see Fig.~\ref{fig:kagome}). Note that vectors $\mathbf{D}_{ij}=D^{[z]}\hat{z}+\mathbf{D}_{ij}^{[R]}$
have an in-plane Rashba-like component $\mathbf{D}_{ij}^{[R]}$ directed
orthogonally to bonds and outwards with respect to bond triangles
(see Fig.~\ref{fig:kagome}). The Rashba-like DMI could result from
mirror asymmetry with respect to the kagome planes. At sufficiently
low temperatures the Hamiltonian in Eq.~(\ref{eq:Ham}) can be analyzed
by applying the Holstein-Primakoff transformation. The corresponding
magnon spectrum is shown in Fig.~\ref{fig:kagome} where the lower,
middle, and upper bands have the Chern numbers $-1$, $0$, and $1$,
respectively.
\begin{figure} \centerline{\includegraphics[clip,width=1\columnwidth]{kagome}}
\protect\caption{(Color online) Left: A two-dimensional kagome lattice with lattice vectors ${\bf a}_1=\frac{1}{2}(\sqrt3,-1)$ and ${\bf a}_2=\frac{1}{2}(\sqrt3,1)$ where atoms are placed in the corners of triangles. Rashba-like DMI vectors $\mathbf{D}_{ij}^{[R]}$  are shown by blue vectors perpendicular to the bonds. The clockwise ordering of bonds corresponding to $\nu=1$ is shown by black arrows. Right:  Magnon spectrum of a kagome ferromagnet with DMI $D^{[z]}=0.3J$ and magnetization pointing in the $z-$ direction. The distribution of the Berry curvature over the Brillouin zone is plotted by the color coding on top of the spectrum for each subband. }
\label{fig:kagome}
\end{figure}

We begin by analyzing an effect of magnon pumping by magnetization
dynamics. This effect is characterized by tensor $\boldsymbol{\alpha}_{\alpha}$
or equivalently by Eq.~(\ref{eq:pumping}). It is also clear from
Eq.~(\ref{eq:Onsager}) that the same tensor also describes a magnetization
torque induced by an analog of electric field for magnons. We assume
a small-angle precession of magnetization around the $z-$ axis. By
symmetry consideration, it is sufficient to consider only $\alpha_{yx}^{\text{even}}=-\alpha_{xy}^{\text{even}}$
and $\alpha_{xx}^{\text{odd}}=\alpha_{yy}^{\text{odd}}$ components
of the tensor where we separate tensor $\boldsymbol{\alpha}_{\alpha}$
into the parts that are odd and even under magnetization reversal,
i.e., $\boldsymbol{\alpha}_{\alpha}=\boldsymbol{\alpha}_{\alpha}^{\text{odd}}+\boldsymbol{\alpha}_{\alpha}^{\text{even}}$.
The results of our calculations for the two components are shown in
Fig.~\ref{fig:alpha}. Note that we use a simple phenomenological
treatment by relating the quasiparticle broadening to the Gilbert
damping as $\Gamma=\alpha\hbar\omega$. Under a simple circular precession
of the magnetization described by angle $\theta$ we have $\partial_{t}\mathbf{m}=\theta\omega[-\sin(\omega t),\cos(\omega t),0]^{T}$
and
\begin{equation}
\begin{array}{c}
J_{px}=\theta\omega[\alpha_{xx}^{\text{odd}}\cos(\omega t)-\alpha_{yx}^{\text{even}}\sin(\omega t)],\\
J_{py}=\theta\omega[\alpha_{xx}^{\text{odd}}\sin(\omega t)+\alpha_{yx}^{\text{even}}\cos(\omega t)].
\end{array}\label{eq:ac-current}
\end{equation}
We can now estimate the amplitude of ac spin current as $\theta\hbar\omega\sqrt{(\alpha_{xx}^{\text{odd}})^{2}+(\alpha_{yx}^{\text{even}})^{2}}$.
For a three-dimensional system containing weakly interacting kagome
layers, we can write $\alpha_{ij}^{\text{3D}}=\alpha_{ij}^{s}/c$
where $c\propto \text{a}_0$ is the interlayer distance which is comparable
to the lattice constant $\text{a}_0$. For parameters $D^{[z]}=0.1J$, $D^{[R]}=0.1J$,
$\theta=0.1\degree$, $\omega=2\pi\times10$GHz, $k_{B}T=0.5SJ$,
and the Gilbert damping $\alpha=0.1$, we obtain the spin current
of amplitude $J_{s}\approx10^{-8}$J/m$^{2}$. We suggest to detect
such spin currents by the ac inverse spin Hall effect \cite{Weiler.Shaw.ea:PRL2014}.
\begin{figure} \centerline{\includegraphics[clip,width=1\columnwidth]{fig2}}
\protect\caption{(Color online) Left: The odd component of the tensor $\alpha_{ij}$ as a function of temperature. The plot is rescaled by multiplying it with the Gilber damping $\alpha$. Right:  The even component of the tensor $\alpha_{ij}$ as a function of temperature. In both cases the magnetization is along the $z-$ axis. For the strength of the Rashba DMI we use $D^{[R]}=D^{[z]}=D$. }
\label{fig:alpha}
\end{figure}\begin{figure} \centerline{\includegraphics[clip,width=1\columnwidth]{fig1}}
\protect\caption{(Color online) Left: The odd component of the torkance tensor $\beta_{ij}$ as a function of temperature. The plot is rescaled by multiplying it with the Gilber damping $\alpha$. Right:  The even component of the torkance tensor $\beta_{ij}$ as a function of temperature. In both cases the magnetization is along the $z-$ axis. For the strength of the Rashba DMI we use $D^{[R]}=D^{[z]}=D$. }
\label{fig:beta}
\end{figure}

We also consider an effect of heat pumping by magnetization dynamics.
This effect is characterized by tensor $\boldsymbol{\beta}_{\alpha}$.
Here we again assume a small-angle precession of magnetization around
the $z-$ axis. Similar symmetry considerations result in relations
$\beta_{yx}^{\text{even}}=-\beta_{xy}^{\text{even}}$ and $\beta_{xx}^{\text{odd}}=\beta_{yy}^{\text{odd}}$
between non-zero components of tensor $\boldsymbol{\beta}_{\alpha}=\boldsymbol{\beta}_{\alpha}^{\text{odd}}+\boldsymbol{\beta}_{\alpha}^{\text{even}}$
separated into the odd and even under magnetization reversal parts.
The results of our calculations for the two components are shown in
Fig.~\ref{fig:beta}. The amplitude of ac heat current is given by
$\theta T\omega\sqrt{(\beta_{xx}^{\text{odd}})^{2}+(\beta_{yx}^{\text{even}})^{2}}$
which for the above parameters and $T=50$K results in the heat current of amplitude
$J_{q}\approx50$kW/m$^{2}$.

After invoking the Onsager relation (\ref{eq:Onsager}) one can confirm that estimates obtained in this subsection are comparable to estimates for thermal torques obtained in Ref.~\cite{Kovalev.Zyuzin:PRB2016}. Note also that the phenomenology discussed in this paper is similar to
Ref.~\cite{Freimuth.Bluegel.ea:JPCM2016}, however, the heat current
is carried by magnons in contrast to electronic mechanisms considered
before.

\section{Conclusions}

In this work, we explored fictitious electric fields acting on magnons in response to time-dependent magnetization dynamics in the presence of DMI. We find that such fictitious electric fields can drive sizable spin and energy currents. We suggest a detection scheme relying on the ac inverse spin Hall effect \cite{Weiler.Shaw.ea:PRL2014}. Additionally, we obtain an analog of the Hall-like response in systems with non-trivial Berry curvature of magnon bands. This leads to even under magnetization reversal contributions to the response tensors. By the Onsager reciprocity relation, this Hall-like response can be related to the anti-damping thermal torque \cite{Kovalev.Zyuzin:PRB2016}. Finally, we identify the ground state energy current associated with the magnon-mediated equilibrium contribution to DMI. This contribution needs to be subtracted from the Kubo linear response result according to our analysis.

\vspace{0.2in}

\begin{acknowledgments}

We gratefully acknowledge useful discussions with K.~Belashchenko. This work was supported by the U.S. Department of Energy, Office of Science, Basic Energy Sciences, under Award No. DE-SC0014189.
\end{acknowledgments}

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text:
//
//  UIView+RBLayout.h
//  Pods
//
//  Created by baxiang on 2017/2/13.
//
//

#import <UIKit/UIKit.h>

@interface UIView (RBLayout)
@property(nonatomic) CGFloat            left;   /** 左 */
@property(nonatomic) CGFloat            top;    /** 上 */
@property(nonatomic, readonly) CGFloat  right;  /** 右 */
@property(nonatomic, readonly) CGFloat  bottom; /** 下 */
@property(nonatomic) CGFloat            width;  /** 宽度 */
@property(nonatomic) CGFloat            height; /** 高度 */
@end

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