Chaitanya Impex, was established in the year 2008 and is a reputed name in the textile industry. Our range has been widely appreciated by our clients' from all walks of society and have superior quality features that conform to international quality parameters.
We are renowned manufacturers and suppliers of an appreciative range of Apparel fabrics and Textile fabrics that can be customized as per clients' specifications. Since the time of inception, we have established fruitful relationships with our clients' and strive, canvas fabrics, cotton canvas supplier, drill fabric suppliers, cotton drill fabrics, twill fabric supplier, cotton twill fabrics, cotton duck fabric, voile fabric supplier hard to attain maximum clients' satisfaction.
Our state-of-the-art infrastructure unit boasts of the latest machines and other technological advancements. We have a fully equipped manufacturing facility, R&D unit, testing unit and warehousing and packaging unit which are constantly upgraded every now and then. Moreover, our team members work together and ensure that the range offered to our clients is of utmost quality at all levels. The team at Chaitanya Impex is led by our mentor and proprietor Mr. Tarang Gupta and our annual turnover has gone up to US$ 0.25-1 Million (or Rs. 1-4 Crore Approx.) in the year 2010-11.
We are one of most reputed manufacturers and suppliers of a vast range of Apparel fabrics and Textile Fabrics. Our product range includes Cambric Fabrics, Poplin Fabrics, Export Yarn Dyed Fabrics, Voile Fabrics, Drill Fabrics, Canvas Fabrics, Pocketing Fabrics, Twill Fabrics, Air Mesh and Duck Oxford Weave, to name only a few.
At Chaitanya Impex, we have a highly qualified team of professionals who work round the clock and ensure that only quality products are dispatched in order to attain maximum clients satisfaction.
We provide them with a congenial environment to work in and train them on the various aspects of the new technology developments. They work as a team and strive hard towards achieving the long-term vision of the company.


text:
For PhD's
Study portals
Staff portal - CC (in Danish)
Centre for Studies in Otherness
You are here: Front Page Past Projects Student Seminar Session
Student Seminar Session
Postgraduate Symposium in Limerick, Ireland
Otherness and Evil: Research Symposium and Book Launch
Otherness: A Multilateral Perspective
Otherness: Essays and Studies
The Centre for Studies in Otherness hosted a Student Seminar evening on the 7th of June, 2011 at Aarhus University.
This session was part of our ongoing seminar series on Otherness and included 30 minute presentations from our student speakers:
Laura Helene Hechmann (Institute for Language, Literature and Culture, AU): You, the Other and dust. Dust as a literary and philosophical symbol
This presentation discussed ethical issues relating to the concept of dust as a literary and philosophical symbol. Focusing on counterpointing concepts such as destruction and character definition, it analysed selected passages from 'The Waste Land' by T.S Eliot and 'The Duchess of Malfi' by John Webster with a view to furthering an ethical theory of our human relationship to the Otherness of death.
Ian Rynne (Institute for Psychology, AU): Synaesthesia, Perception and Otherness
Historically, it was widely considered that the world presents itself to our senses in a uniform way. The implication of this view is that the common phenomenological experience of perception is the correct one. The minority of individuals who reported consistent but unusual sensory experiences and connections (i.e. Synaesthesia) were considered, at worst, to be lunatics and, at best, to be victims of rare and troublesome crossing of the senses. This primarily empirical presentation showed some examples of how the phenomenology of synaesthetic perception can differ from the norm. However, it also demonstrated how it is not nearly rare as previously thought and how it is most likely a constituent part of "normal" perception. The world we see, hear and smell every day is, primarily, a dynamically changing construction, subject greatly to individual difference but constrained by experience. Hopefully we can then discuss what implications this has for basic conceptions of the Same and the Other.
5427 / i33

redpajama_set_name: RedPajamaCommonCrawl


text:
SHIELDS Agnes
Name SHIELDS Agnes [1, 2]
Born Bef 8 Oct 1843 Torphichen, West Lothian, Scotland [3, 4]
Christened 8 Oct 1843 [1]
Census 1871 Torphichen, West Lothian, Scotland [3]
Census 1881 Strathloanhead, Torphichen, Linlithgow, Scotland [5]
aged 37, married
Census 1901 Strathloanhead, Torphichen, West Lothian, Scotland [3, 4]
Residence 1905 Strathloanhead, Torphichen, West Lothian, Scotland [6]
aged 65, possible
Died 17 Mar 1921 Torphichen, West Lothian, Scotland [1, 3]
Person ID I19 Mastertons from Bathgate (1)
Father SHIELDS William
Mother MARSHALL Jane
Married 19 Nov 1837 [1]
Family MASTERTON James, b. Bef 3 Jun 1841, Bathgate, West Lothian, Scotland , d. 5 Aug 1925, Royal Infirmary, Edinburgh, Scotland (Age > 84 years)
Married 21 Feb 1868 Torphichen, West Lothian, Scotland [1, 3]
1. MASTERTON Jean (Jane) Marshall, b. 31 Aug 1868, Torphichen, West Lothian, Scotland , d. 1928, Torphichen, West Lothian, Scotland (Age 59 years)
2. MASTERTON Margaret Arthur, b. 1870, Torphichen, West Lothian, Scotland , d. 1960, Linlithgow, West Lothian, Scotland (Age 90 years)
3. MASTERTON Agnes, b. 1872, Torphichen, West Lothian, Scotland , d. 19 Jul 1913, Edinburgh Infirmary, Edinburgh, Midlothian, Scotland (Age 41 years)
4. MASTERTON Elizabeth, b. 1874, Torphichen, West Lothian, Scotland , d. 6 Jan 1955, St Andrew, Edinburgh, Midlothian, Scotland (Age 81 years)
5. MASTERTON Robert, b. Bef 3 Mar 1881, Torphichen, West Lothian, Scotland
[S6] 1881 British Census Chart, David Masterton, Whippany, New JErsey.
[S1] scotlandspeople, General Registers of Scotland.
[S23] Scotland 1901 Census.
[S7] 1881 Census.
[S97] Valuation Roll 1905, scotlandspeople.
[S36] 1911 Scotland Census.
[S96] Valuation Roll 1915, scotlandspeople, (1915).


text:
Q: Why does `rsync` not require super-user privileges? From manpage of rsync:

Some of the additional features of rsync are:

*

*does not require super-user privileges

Is it correct that what rsync process needs is

*

*read permission on every source file,

*and write permission on every destination file?

Any thing incorrect or missing?
Why does the manpage say that rsync "does not require super-user privileges"?
Thanks.

A: Because it's not a daemon, works as long as you have permissions to read (origin) and write (destination) as you stated, and it (somewhat) allows you to preserve ownership/attributes in the copy, even if you are not root or the user at the destination machine (read about --super and --fake-super, for this to work the destination has to be compatible with the ACLs).
From the same manpage of rsync:
 --fake-super
      When this option is enabled, rsync simulates super-user  activi‐
      ties  by  saving/restoring the privileged attributes via special
      extended attributes that are attached to each file (as  needed).
      This  includes  the  file's  owner  and  group (if it is not the
      default), the file's device info (device  &  special  files  are
      created  as  empty  text files), and any permission bits that we
      won't allow to be set on the real file (e.g.  the real file gets
      u-s,g-s,o-t  for  safety) or that would limit the owner's access
      (since the real super-user can always access/change a file,  the
      files  we  create can always be accessed/changed by the creating
      user).  This option also handles ACLs (if --acls was  specified)
      and non-user extended attributes (if --xattrs was specified).

      This  is  a  good way to backup data without using a super-user,
      and to store ACLs from incompatible systems.

Edit and to clarify: "Does not require super-user privileges" doesn't mean it's not useful to be super-user. It just means it will work (mostly) anyway.

redpajama_set_name: RedPajamaStackExchange


This is a big one. Over 3 years of podcasting, I'd have to say this is one of the biggest shows yet. I have a 3 minute interview with the one and only Jimmy Pardo of the Never Not Funny podcast, one of my all time favorite comedians. We also do the Bean Boozle challange where jelly beans could taste great or like garbage, Taylor tells us her idea for a 21 Pilots theme park, the dogs attack with chemical weapons, I read some terrible ideas for teenagers from Indy100, a movie from The Rock saves a child, more national news and an email from a listener leads Jani to drop a bombshell that only about 5 people knew about me, which then leads us to another story I've kept from the public since our first year of marriage.
The headliner for Jimmy Pardo was Matt Donaher.


text:
Charles Malsbury
B.A. Northwestern, M.A., Ph.D. McGill
Email: malsbury@play.psych.mun.ca
Affiliations: Behavioural Neuroscience
General Research Q.: How do gonadal hormones affect brain and behavior? Interests include: neural and endocrine determinants of reproductive and other social behaviors, sex differences in brain structure and function, trophic effects of hormones on brain structure, neuroanatomy (hypothalamic and limbic), neuropeptides, neuroendocrinology.
Most of my research has been aimed at developing a greater understanding of CNS mechanisms regulating mammalian reproductive behavior. Reproductive behaviors are intrinsically interesting but also provide examples of how hormones can change brain and behavior (plasticity). Gonadal hormones (estrogen and testosterone) change the brain by acting on hormone receptors (estrogen and androgen receptors) in particular regions of the brain. Recently I have been studying androgen receptors (ARs). Although ARs are found in areas of the brain important for reproductive behavior, such as the hypothalamus and amygdala, they are also abundant in the hippocampus, a structure important for learning and memory. What are ARs doing in the hippocampus? I have been collaborating with Drs. Doris Babstock and Carolyn Harley on experiments that begin to answer this question.
Hebbard, P.C., King, R.R., Malsbury, C.W. & Harley, C.W. (2003). Two organizational effects of pubertal testosterone in male rats: Transient social memory and a shift away from long-term potentiation following a tetanus in hippocampal CA1. Experimental Neurology, 182:470-475.
Malsbury, C.W. (2002). Hypothalamus. In Encyclopedia of Cognitive Science, Macmillan Reference Ltd.: London (brief review).
Harley, C.W., Malsbury, C.W., Squires, A., & Brown, R.A. (2000). Testosterone decreases CA1 plasticity in vivo in gonadectomized male rats. Hippocampus 10(6):693-7.
Babstock, D., Malsbury, C.W. & Harley, C.W. (1997). The dorsal locus coeruleus is larger in male than in female Sprague-Dawley rats. Neuroscience Letters, 224: 157-160.
Kerchner, M., Malsbury, C.W., Ward, O.B. & Ward, I.L. (1995). Sexually dimorphic components of the medial amygdala are resistant to the demasculinizing effect of prenatal stress. Brain Res., 672: 251-260.
Malsbury, C.W. & McKay, K. Neurotrophic effects of testosterone on the medial nucleus of the amygdala in the adult male rat. J. Neuroendocrinology, 6: 57-69, 1994.


text:
HomeAcademyTrainings1-14 July 2019 - Wimbledon Lawn Tennis Championships
1-14 July 2019 - Wimbledon Lawn Tennis Championships
Industry: Sport, tourism
Dates: 1-14 July 2019
Venue: Wimbledon
Wimbledon, is the oldest tennis tournament in the world, and widely considered to be the biggest and the most prestigious. It has been held at the All England Club in Wimbledon, London since 1877. It is one of the four Grand Slam tennis tournaments, the other three majors being the Australian Open, French Open and US Open. Wimbledon is the only Major still played on grass, the game's original surface, which gave the game its original name of "lawn tennis".
The five main events: Gentlemen's Singles, Ladies' Singles, Gentlemen's Doubles, Ladies' Doubles, Mixed
The four junior events: Boys' Singles, Girls' Singles, Boys' Doubles, Girls' Doubles, Disabled Doubles
The five invitational events: Gentlemen's Invitation Doubles, Senior Gentlemen's Invitation Doubles, Ladies' Invitation Doubles, Gentlemen's Wheelchair Doubles, Ladies' Wheelchair Doubles
Tennis fans
For visiting the conference, please contact the Training Programme Office of BBA UK


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text:
Kleiner Schmetterling (jap. , Ritoru Batafurai, von engl. Little Butterfly) ist eine abgeschlossene Manga-Serie der japanischen Zeichnerin Hinako Takanaga. Sie umfasst über 500 Seiten, wurde in Japan von 2001 bis 2004 veröffentlicht und lässt sich dem Genre Boys Love zuordnen.

Handlung
Der einzelgängerische und erwachsen wirkende Atsushi Nakahara ist ein Außenseiter, was an seinem abweisenden kühlen Verhalten liegt, das er gegenüber seinen Mitschülern auf der Mittelschule in Tokio an den Tag legt. Dies weckt jedoch das Interesse seines beliebten und etwas naiven Schulkameraden Yuki Kojima. Auf einer Klassenfahrt versucht Nakahara wegen seiner schwierigen Familienverhältnisse nach Korea zu flüchten. Nachdem er die hohen Erwartungen seiner Mutter, die ihn auf eine Privatschule schicken wollte, nicht erfüllen konnte, wurde diese immer neurotischer, und Nakaharas Eltern stritten sich oft. Er lief oft davon, kam jedoch nie weit, und sein Vater schenkte ihm immer weniger Beachtung. Kojima will ihm bei seiner Flucht helfen, aber sie verlaufen sich und die Flucht scheitert. Doch kommen sie sich so näher, und Kojima gelingt es, eine Freundschaft zu Nakahara aufzubauen. Sie lernen sich besser kennen, und auch zu Kojimas Freunden gewinnt Nakahara nun ein besseres Verhältnis.

Eines Abends tröstet Kojima Nakahara, nachdem sich dieser wieder mit seiner Mutter gestritten hat, und Nakahara gesteht seine Liebe zu Kojima. Dieser ist aber verunsichert, und nur langsam kommen sie sich näher. Schließlich entscheidet er sich dafür, mit Nakahara gemeinsam auf eine Oberschule mit Internat zu gehen. Als Nakaharas Onkel Ikuo Sugisaki aus Osaka sie besucht, beschließt dessen Schwager, dass er durch seine Firma die erbetene finanzielle Unterstützung gewährt und er dafür seine Frau und seinen Sohn aufnehmen soll. Ikuo stimmt schließlich zu, Nakahara entscheidet sich nach Kojimas Bitten aber dennoch dafür, mit ihm auf das Internat zu gehen. Schließlich haben sie das erste Mal gemeinsam Sex. Doch vor der Aufnahmeprüfung haben sie bald kaum noch Zeit füreinander, und Nakahara geht für kurze Zeit nach Osaka. Dort muss er erfahren, dass es seiner Mutter, nachdem sie von ihrer Scheidung erfahren hat, deutlich schlechter geht. Nach der Prüfung kehrt er gleich wieder nach Osaka zurück, seine Mutter hat inzwischen vergessen, dass er ihr Sohn Atsushi ist. Sie glaubt, ihr Sohn würde im Ausland studieren, und wartet auf dessen Rückkehr. Sie erzählt Atsushi immer wieder von diesem Sohn, der sich dann ebenso in diesen Vorstellungen verliert. Doch Kojima vermisst Nakahara sehr und reist schließlich zu ihm nach Osaka. Erst durch ihn und die nun gegenseitige Liebe kann sich Nakahara von seiner Mutter lösen und fährt mit seinem Geliebten zurück nach Tokio. Dort besuchen beide die Abschlussfeier der Mittelschule und freuen sich auf die gemeinsame Zeit auf der Oberschule.

Veröffentlichungen
Kleiner Schmetterling erschien in Japan von 2001 bis 2004 in Einzelkapiteln im Manga-Magazin Gush, das vom Kaiosha-Verlag herausgegeben wird und sich auf Liebesgeschichten zwischen homosexuellen Männern spezialisiert hat. Der Verlag brachte die etwa 400 Seiten umfassenden Einzelkapitel auch in drei Sammelbänden heraus.

Der Manga wurde unter anderem ins Englische und Deutsche übersetzt.

Auf Deutsch wurden die drei Bände von August 2005 bis Januar 2006 von Tokyopop veröffentlicht. Der erste Band stand im August 2005 auf Platz vier und im September 2005 auf Platz zehn der monatlichen Manga-Verkaufscharts in deutschen Buch- und Comicläden; der zweite Band kam im Oktober 2005 auf Platz drei und November 2005 auf den fünfzehnten Rang; der dritte Band kam im Januar 2006 auf den dritten Platz. Im März 2007 wurde der komplette Manga erneut als Einzelband herausgebracht. Aufgrund des Erfolgs der Serie veröffentlichte Tokyopop weitere Werke von Hinako Takanaga.

Von Hinako Takanaga erschien auch das Artbook Kleiner Schmetterlin & mehr, das im Juni 2014 auch auf Deutsch herauskam.

Weblinks
 Website des deutschen Manga
 Anime News Network über den Manga (englisch)

Manga (Werk)
Homosexualität im Manga

redpajama_set_name: RedPajamaWikipedia


text:
How to Get Masters Tickets
Famous Golfers
You'll Need Some Luck -- and a Lot of Money
Andrew Redington/Getty Images
by Brent Kelley
Brent Kelley is an award-winning sports journalist and golf expert with over 30 years in print and online journalism.
If you've been lucky enough to attend a Masters Tournament, no doubt you want to go back. And if you've never been, then you're probably already dreaming of heading to Augusta National for the next one.
Masters tickets aren't impossible to find, but they are among the toughest tickets in all of sports to get. And if you are able to find Masters tickets, it will probably require a lot of money — perhaps even thousands of dollars — to purchase one.
But there is some good news: In 2012, Augusta National Golf Club began making a (very) small number of tournament tickets available for purchase through a random drawing following online registration. The club also changed how it handles practice-round ticket requests, requiring all ticket-seekers to register online (abandoning the old mail-in process).
Prior to those announcements, tickets to tournament days (rounds one through four) had not been available from the Masters Tournament directly to the general public since 1972. That year, Augusta National Golf Club opened a waiting list, but due to demand, the waiting list itself had to be closed in 1978. Twenty-two years later, in the year 2000, a new waiting list was opened, but it is now also closed.
There are options, however; some of them relying on luck and all of them requiring a good bankroll. The options are much more limited for tournament days, but open up a bit for passes to Masters practice days.
Key Takeaways: Masters Tickets
Tickets to The Masters Tournament are among the most difficult to get tickets in all of sports.
Prices of Masters tickets listed by ticket brokers can easily reach into the thousands of dollars for tournament rounds.
Augusta National Golf Club runs The Masters and also runs a ticket lottery. The lottery awards tickets to practice days before the start of the tournament, plus a very small number of tickets for tournaments rounds.
To create an account, take part in the ticket lottery, and be notified annually, visit the tickets section of the Masters' official website.
Masters Tournament Tickets
Masters badges are "among the most coveted tickets for any event, sporting or otherwise," according to Brian Talbot of TickCo Premium Seating.
"From my experience, it's safe to say these are probably the toughest tickets to get in the world," Talbot said, "with Super Bowl tickets running a close second, depending on which teams make it and where the Super Bowl is hosted."
But there is a tiny window through which fans can obtain Masters tickets for tournament rounds directly from Augusta National. Each year, a small number of tickets are returned to The Masters following the deaths of longtime ticketholders, or for other reasons. Previously, those tickets were simply removed from circulation. But since 2012, fans can register online to take part in a random drawing for those tickets.
To do so, golfers much register on the tickets page on Masters.com; registrants receive notification when the ticket application process is opened each year, shortly following each Masters. Registrants are required to provide credit card information during the online application process.
The Masters doesn't say how many tournament tickets are available, but rest assured the number is very small and your odds are very, very long. Those who are super-lucky are notified by email and must pay for the tickets at such time.
But if you're not among the super-lucky who get those tickets, what other options exist for golf fans desperate to attend The Masters during tournament play? Ticket brokers are the easiest route since many ticket brokers have been buying tickets from Masters ticketholders for years. But those tickets are hugely expensive. Tournament badges at ticket brokers might begin around $1,500 and can soar as high as $12,000 for a single ticket.
As with any major purchase, shop around among different ticket brokers to see if you can find a good deal (comparatively speaking of course). Your best bet is to buy early if you're going the ticket broker route since brokers have a limited supply. The larger, most established brokers might have 100 tickets available, while smaller brokers may have only one or two.
The auction giant eBay is another option, although you're more likely to find practice tickets than tournament tickets that way.
And you can always simply show up outside the Augusta National gates and hope to get lucky with a scalper. Ticket scalping was legalized in 2001 by the Georgia Legislature so long as the sale occurs at least 1,500 feet away from the event site. However, you can be the unfortunate recipient of a fraudulent ticket if you use this method to obtain tickets, so be careful when buying.
Masters Practice Tickets
Tickets to Masters practice days are much easier to come by than tournament badges, although you'll still need a little luck and a good amount of cash.
Practice tickets are more readily available through brokers and on eBay, but the good news is that Masters practice-day tickets are available for purchase by the general public from The Masters itself. A limited number of practice tickets are sold in advance by The Masters, by online application only. Whether you get tickets — and how many you get — is the result of a random allocation among all applicants. But your odds of getting Masters tickets for practice rounds are much, much better than getting tournament tickets.
Practice round tickets from The Masters have face values of $75. If you have to buy through a ticket broker, you'll likely pay several hundred dollars for Monday and Tuesday tickets, perhaps more than $1,000 for Wednesday tickets (because of the Par-3 Contest).
Go to the tickets page on Masters.com and follow the online registration/application process. The application for next year's Masters usually opens a month or two after this year's Masters concludes, but register early to make sure you don't miss out on the opportunity. Following a random drawing to allocate the practice-day tickets, lucky golfers are notified by email and must pay at that time.
You Only Have to Register Once at Masters.com
If you've registered at Masters.com for previous year ticket drawings, you don't need to do it again. Once you're in the system, you'll receive a notification when the next ticketing process begins.
Have questions about the Masters' own ticketing process? The Masters Tournament ticket office can be reached by phone for more information.
2 (Relatively) Easy Ways to Get PGA Championship Tickets
The Changing Process for Obtaining Super Bowl Tickets
Find Out When the 2020 Masters Golf Tournament Takes Place
What You Need to Know About the 2020 U.S. Open Tournament
How You Can Get Tickets to the U.S. Open
How Much Does It Cost to Join Augusta National—and Who Are Members?
What You Should Know About Augusta National Women's Amateur Tournament
Yes, You Can Enter a US Open Qualifier — Here's How
Tour the Famous Landmarks at Augusta National Golf Club
The 7 Tournaments Where Arnold Palmer Made the Biggest Impact on Golf
The Basics on Golf Club Sets
Here's How the USGA Decides on the Pairings for the US Open Tournament
Discount Broadway Theater Clubs
Biography of Legendary Golfer Bobby Jones, a Giant of the Sport
7 Times Golfers Ripped the USGA Over the US Open Golf Course
Golf Betting Games and Tournament Formats Explained


text:
Reading is getting its first ever Taco Bell
The new restaurant is going to replace a shoe store
Alex Seabrook
Taco Bell is opening its first restaurant in Reading (Image: Peter Harbour)
Taco Bell has received permission to open its first restaurant in Berkshire.
The American chain has applied for permission to open a new outlet in the Broad Street Mall, which has been granted by Reading Borough Council.
Taco Bell will go next to the Metro Bank, where Footlocker used to be in Oxford Road.
It is still unclear when the restaurant will open, although they are already hiring staff and in the process of converting the unit.
The restaurant has worked with the council on detailed plans regarding ventilation, smell and litter.
Reading restaurant launches roast dinner pizza
In the meantime there are already Taco Bells in Woking, Southampton, London, Bournemouth, Chichester, and several other places across the UK.
We previously reported the Mexican chain was looking for a general manager and a shift manager, before planning permission was granted.
If you are looking for work in Reading, there are 128 jobs available in the town on Fish4Jobs now.
It is also recruiting team members and a supervisor for the restaurant.
It was revealed the company is coming to Reading in September - it will be the company's first restaurant in Berkshire.
Anyone interested in any of the roles can find out more or apply here.
ldrcontent
MaidenheadHelen Glover and Steve Backshall welcome baby twins in adorable Instagram postThe Olympic gold medal winner and TV presenter, who live near Maidenhead, asked for advice on how to look after three children under three
NewburyTopshop in Newbury to close this yearA closing date has been set as Topshop Topman reveals it is pulling out of the Berkshire town
After DarkNew plans emerge to replace Reading's After Dark club with flatsThe London Street club could be forced to close at the end of the month


text:
Антон Бонавентура Еглич (, 29.05.1850 г., Австро-Венгрия — 1.07.1937 г., Любляна, Югославия) — католический прелат, епископ Любляны с 24 марта 1898 года по 17 мая 1930 год, словенский общественный деятель.

Биография
После изучения теологии Антон Бонаветнура Еглич 27 июля 1873 года был рукоположён в священника, после чего продолжил своё обучение в Вене. После возвращения на родину Антон Бонавентура Еглич был капелланом в женской тюрьме. Позднее изучал теологию в Италии и Германии, после чего был преподавателем в люблянской семинарии.

13 августа 1897 года Римский папа Лев XIII назначил Антона Бонавентуру Еглича титулярным епископом Сиунии и вспомогательным епископом архиепархии Врхбосны. 12 сентября 1897 года состоялось рукоположение Антона Бонавентуры Елича в епископа, которое совершил архиепископ Врхбосны Йосип Стадлер. 24 марта 1898 года был назначен епископом Любляны.

Антон Бонавентура Еглич активно занимался общественной и просветительской деятельностью среди словенцев в период с 1898 по 1930 год. По его инициативе была издана первая полная словенская грамматика. Он же содействовал учреждению первой полноценной словенской гимназии в люблянском предместье Шентвиде (Šentvid).

В 1899 г., по приказу Еглича, был скуплен и сожжён почти весь тираж книги стихов Ивана Цанкара «Эротика».

Еглич имел большой авторитет среди членов Католической народной партии (Katoliško narodno stranko, SLS). В годы Первой мировой войны Антон Бонавентура Еглич занял резко-антисербскую позицию. Выступая 11 августа 1914 года перед солдатами-словенцами, он восклицал:

В марте 1917 года Еглич призвал к расширению автономии Словении и других национальных земель Австро-Венгрии; вскоре он поддержал Майскую декларацию Антона Корошеца.

17 мая 1930 года Антон Бонавентура Еглич вышел в отставку и был назначен Святым Престолом титулярным архиепископом Гареллы (Gornji Grad). В 1932 г. переведён в Стично (Stično).

Скончался 1 июля 1937 года в Любляне. Незадолго до смерти, 29 июня 1937 г., Еглич произнёс речь против безбожия и коммунизма.

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Католические епископы Словении


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On Wednesday the 20th of June, whilst in Cape Verde, island of Sal, I did a days dive. Dived with a company called Atlantic Star, I thought they were a professional set up.
My first dive I did, was a wall dive about depth about 20 meters, place called Pontinha, there was 4 divers and the guide, nice Reef to dive along and plenty of corals and marine life.
The second dive was a wreck called Santo Antao, just myself and the guide on that dive, what was great, depth was about 10 meters, loads of marine life again, plenty of puffer fish, various sizes, both dives were just under the hour, to get to dive sites was from a rib, so backwards roll entry, Guide commented on my awareness, helpfulness and diving, said was good, that was all down to my club, Harlow BSAC club.


text:
\section{Introduction}\label{sec:introduction}
The nature of the $\Lambda(1405)$ has been in dispute since the early days. In
most quark-model calculations, it is described as a $p$-state $q^3$ baryon with
mainly a SU(3) singlet structure~\cite{Isgur:1978xj}.  On the other hand, the $\Lambda(1405)$
resonance has long been suggested to be a bound state of the $\bar{K}N$ system,
and therefore of $q^4\bar{q}$ structure~\cite{Dalitz:1960du}.  In recent years,
this argument has been strengthened within the unitary extensions of chiral
perturbation theory
U$\chi$PT~\cite{Kaiser:1996js,Oset:1997it,Oset:2001cn,Oller:2000fj,Jido:2003cb,Garcia-Recio:2002td,Garcia-Recio:2003ks,Hyodo:2002pk}.
A particularly interesting discovery is that the nominal $\Lambda(1405)$ is a
superposition of two resonances. This was hinted in \cite{Oller:2000fj}
and studied in detail in \cite{Jido:2003cb}, where two poles were found
on the second Riemann sheet at $1390-i66$\,MeV and
$1426-i16$\,MeV, respectively. More recently, the studies of the $\bar{K}N$ interaction  have
been extended by including higher order chiral Lagrangians in the kernel of
the interaction~\cite{Borasoy:2005ie,Oller:2005ig,Oller:2006jw,Borasoy:2006sr}.
The position of the high-energy pole is rather similar in all these works and in
\cite{Jido:2003cb}, but there are variations in the position of the low-energy
pole. Nevertheless, the theoretical uncertainties have been studied in \cite{Borasoy:2006sr}
and the results of Ref.~\cite{Jido:2003cb} fit well within them.
As first demonstrated in Ref.~\cite{Jido:2003cb}, due to the
fact that these two poles couple differently to the coupled channels, different
reactions could observe different invariant mass distributions, thus offering
the possibility to experimentally test the two-pole prediction. The reactions $\gamma
p\rightarrow K^+\Lambda(1405)$ and $K^-p\rightarrow \Lambda(1405)\gamma$ are
shown to be sensitive to the high-energy pole of the $\Lambda(1405)$ and thus the corresponding
invariant mass distributions
exhibit a peak at $\sim 1420$\,MeV~\cite{Nacher:1998mi,Nacher:1999ni}. On the other hand, the
reaction $\pi^-p\rightarrow K^0\pi\Sigma$ seems to give more
weight to the low-energy pole and thus exhibits a peak around
$1390$\,MeV in the $\pi\Sigma$ invariant mass distributions~\cite{Hyodo:2003jw}. Such a two-pole structure of the
$\Lambda(1405)$ has recently been tested by the reaction
$K^-p\rightarrow\pi^0\pi^0\Sigma^0$~\cite{Prakhov:2004an}, as demonstrated in
Ref.~\cite{Magas:2005vu}.

The electromagnetic transition rates of excited baryons to their respective
ground states provide a relatively clean probe of the structure of the baryons.
In this respect, we expect that the radiative decay widths of the $\Lambda(1405)$
can offer us some clues on its two-pole structure. However, the radiative
decays of the excited hyperon states have very small branching ratios and to
date very few electromagnetic transition rates have been measured. Recently,
the CLAS collaboration at Jefferson Lab has reported a new measurement of the
radiative decay widths of the $\Sigma^0(1385)$ and the
$\Lambda(1520)$~\cite{Taylor:2005zw}, which, as argued in
Ref.~\cite{Myhrer:2006hx}, suggests that the wave functions of the hyperon
ground states should contain sizable components of excited quark states
(configuration mixing). As for the $\Lambda(1405)$, there is no direct
measurement of its radiative decay widths. Using an isobar
model  to fit the $K^-p$ atom data of Ref.~\cite{Whitehouse:1989yi}, H. Burkhardt and J. Lowe ~\cite{Burkhardt:1991ms}
obtained the following numbers:
\begin{eqnarray*}
&&\Gamma_{\Lambda(1405)\rightarrow\gamma\Lambda(1116)}=27\pm8\,\mbox{keV},\\
&&
\Gamma_{\Lambda(1405)\rightarrow\gamma\Sigma^0(1193)}=10\pm4\,\mbox{keV}\quad\mbox{or}\quad
23\pm7\,\mbox{keV},
\end{eqnarray*}
which are sometimes quoted as ``experimental data'' in the literature.

On the other hand, as shown in Ref.~\cite{Lee:1998gt}, the U$\chi$PT
model of Refs.~\cite{Oset:1997it,Oset:2001cn} can also describe
rather well the $K^-p$ atom data of Ref.~\cite{Whitehouse:1989yi}.
Therefore, it is truly desirable to calculate the radiative decay
width of the $\Lambda(1405)$ within the same framework. This is the
main purpose of the present work.

This paper is organized as follows. In Sect.~\ref{sec:cc} we give a
brief description of the chiral unitary coupled channel approach. In
Sect.~\ref{sec:decay} we calculate the radiative decay widths of the
$\Lambda(1405)$, discuss how these numbers are closely related to
the chiral structure of our approach and compare our predictions
with those of other theoretical models. In Sect.~\ref{sec:reaction}
we study the reactions $K^-p\rightarrow
\pi^0\gamma\Lambda(\Sigma^0)$ and $\pi^-p\rightarrow K^0\gamma
\Lambda(\Sigma^0)$. There we show that while the first reaction
stresses the high-energy pole of the $\Lambda(1405)$ in both the
$\gamma\Lambda$ and $\gamma\Sigma^0$ channels, the second reaction
gives more weight to the low-energy pole in the $\gamma\Sigma^0$
channel.  Conclusions and a brief summary are presented in
Sect.~\ref{sec:summary}.

\section{Brief description of the two $\Lambda(1405)$ states in
the chiral unitary coupled channel approach\label{sec:cc}}
 In \cite{Oset:1997it,Oset:2001cn,Oller:2000fj,Jido:2003cb},
 the unitary formalism with coupled channels
 using chiral Lagrangian is exposed. The lowest order chiral
 Lagrangian for the interaction of the pseudoscalar mesons of the SU(3)
 octet of the pion with the baryons of the proton octet is used. By
 picking the terms that contribute to the $MB\rightarrow MB$
 amplitude the Lagrangian is given by \cite{Oset:1997it}:
\begin{equation}
\mathcal{L}=\frac{1}{4f^2}\langle\bar{B}i\gamma^\mu[\Phi\partial_\mu\Phi-\partial_\mu\Phi
\Phi,B]\rangle,
\end{equation}
which, projected over $s$-wave, provides tree level transition
amplitudes \cite{Oset:2001cn}:
\begin{eqnarray}
V_{ij}&=&-C_{ij}\frac{1}{4f^2}(2\sqrt{s}-M_{B_i}-M_{B_j})\nonumber\\
&&\quad\quad\quad\times\left(\frac{M_{B_i}+E}{2M_{B_i}}\right)^{1/2}
\left(\frac{M_{B_j}+E'}{2M_{B_j}}\right)^{1/2},
\end{eqnarray}
with $E$, $E'$ ($M_B$) the energies (masses) of the baryons and
$C_{ij}$ coefficients tabulated in \cite{Oset:1997it}. These tree
level amplitudes are used as kernel of the Bethe Salpeter equation
in coupled channels
\begin{equation}
T=[1-Vg]^{-1}V,
\end{equation}
where $V$ appears factorized on shell
\cite{Oset:1997it,Oller:2000fj} and $g$ is the loop function of a
meson and a baryon propagators, regularized by a cut off in
\cite{Oset:1997it} and in dimensional regularization in
\cite{Oller:2000fj,Oset:2001cn,Jido:2003cb}.

For the particular case of ${1/2}^-$ states (in $MB$ $s$-wave
interaction) with strangeness $S=-1$ and zero charge we have ten
channels: $K^-p$, $\bar{K}^0n$, $\pi^0\Lambda$, $\pi^0\Sigma^0$,
$\eta\Lambda$, $\eta\Sigma^0$, $\pi^+\Sigma^-$, $\pi^-\Sigma^+$,
$K^+\Xi^-$, and $K^0\Xi^0$. The explicit solution of the Bethe
Salpeter equation leads to poles in the second Riemann sheet
corresponding to resonances. In this sector one finds two poles
close to the nominal $\Lambda(1405)$ resonance, and other poles
corresponding to the $\Lambda(1670)$ and other $\Sigma$
resonances~\cite{Oset:2001cn,Jido:2003cb}. The pole position
provides the mass and half width (through its imaginary part) and
the residues at the pole give the couplings of the resonance to the
different channels. These couplings will be needed in what follows
to determine the radiative decay widths of the $\Lambda(1405)$. Only
one loop function involving these latter couplings will be used, but
one has to keep in mind that the resonance couplings used in the
evaluation summarize the effect of the multichannel multiple
scattering of the different states prior to the final coupling to
the photon. Although arguments of gauge invariance require the
coupling of the photon to all internal loops of the diagrammatic
series of the Bethe Salpeter equation~\cite{Borasoy:2005zg}, such
loops involve an $s$-wave and a $p$-wave vertex and vanish in the
present case in the large baryon mass limit. In practice, they are
negligible for finite masses \cite{Doring:2006ub,Doring:2005bx}.

In Table \ref{table:jido} we summarize the pole position and
couplings of the two $\Lambda(1405)$ states to the different
channels. These will be used in the next section. We omit in the
table the neutral channels $\eta\Lambda$, $\eta\Sigma$,  and
$\pi\Lambda$, which do not contribute to the radiative decay of the
$\Lambda(1405)$.

\begin{table}[htpb]
\renewcommand{\arraystretch}{1.5}
\setlength{\tabcolsep}{3mm}
 \centering \caption{\label{table:jido}The two poles $z_R$ of the $\Lambda(1405)$ and the corresponding
 couplings to different coupled channels. Taken from Ref.~\cite{Jido:2003cb}.}
\begin{tabular}{ccccc}
\hline\hline
 $z_R$ & \multicolumn{2}{c}{$(1390-66i)$} & \multicolumn{2}{c}{$(1426-16i)$}\\

    & $g_i$ & $|g_i|$ & $g_i$ & $|g_i|$ \\
    \hline
$\pi\Sigma$ & $-2.5+1.5i $ & 2.9 & $0.42+1.4i$ & 1.5\\
$\bar{K}N$ & $1.2-1.7i$ & 2.1 & $-2.5-0.94i$ & 2.7 \\
$K\Xi$ & $-0.45+0.41i$ & 0.61 & $0.11+0.33i$ & 0.35    \\
 \hline\hline
\end{tabular}
\end{table}

\begin{figure*}[htpb]
 \centering
\includegraphics[scale=0.7]{figure1.eps}
\caption{\label{figure_decayw}The radiative decay mechanism of the
$\Lambda(1405)$, where $MB$ can be any of the four charged channels
of the ten coupled channels:
 $K^-p$, $\bar{K}^0n$,
$\pi^0\Lambda$, $\pi^0\Sigma^0$, $\eta\Lambda$, $\eta\Sigma^0$,
$\pi^+\Sigma^-$, $\pi^-\Sigma^+$, $K^+\Xi^-$, and $K^0\Xi^0$.}
\end{figure*}

 The model of Ref.~\cite{Oset:1997it} was calibrated
 using the following threshold branching ratios:
\begin{eqnarray*}
    \gamma&=&\frac{\Gamma(K^-p\rightarrow\pi^+\Sigma^-)}{\Gamma(K^-p\rightarrow\pi^-\Sigma^+)}
    =2.36\pm0.04,\\
    R_c&=&\frac{\Gamma(K^-p\rightarrow\mbox{charged
    particles})}{\Gamma(K^-p\rightarrow\mbox{all})} =0.664\pm0.011,\\
    R_n&=&
    \frac{\Gamma(K^-p\rightarrow\pi^0\Lambda)}{\Gamma(K^-p\rightarrow\mbox{all
    neutral states})} =0.189\pm0.015.
\end{eqnarray*}

With the same set of parameters, in Ref.~\cite{Lee:1998gt}, the following
branching ratios are obtained:
\begin{eqnarray*} B_{K^-p\rightarrow\gamma\Lambda}&=&1.10\times10^{-3}
    \,(0.86\pm0.16\times10^{-3}),\\
    B_{K^-p\rightarrow\gamma\Sigma^0}&=&1.05\times10^{-3}\,(1.44\pm0.31\times10^{-3}),\\
        R&=&\frac{B_{K^-p\rightarrow\gamma\Lambda}}{B_{K^-p\rightarrow\gamma\Sigma^0}}
        =1.04 \,(0.4\sim0.9),
\end{eqnarray*}
which are all in reasonable agreement with the data (shown in the
parentheses)~\cite{Whitehouse:1989yi}. We have made use of this model~\cite{Oset:1997it} and have
evaluated the branching ratios for other reactions as shown below:
\begin{eqnarray*}
R_{\pi^0\Lambda}&=&\frac{\Gamma(K^-p\rightarrow\pi^0\Lambda)}{\Gamma(K^-p\rightarrow\mbox{all})}
=0.083\,(0.075),\\
R_{\pi^0\Sigma^0}&=&\frac{\Gamma(K^-p\rightarrow\pi^0\Sigma^0)}{\Gamma(K^-p\rightarrow\mbox{all})}
=0.293\,(0.261),\\
R_{\pi^+\Sigma^-}&=&\frac{\Gamma(K^-p\rightarrow\pi^+\Sigma^-)}{\Gamma(K^-p\rightarrow\mbox{all})}
=0.437\,(0.467),\\
R_{\pi^-\Sigma^+}&=&\frac{\Gamma(K^-p\rightarrow\pi^-\Sigma^+)}{\Gamma(K^-p\rightarrow\mbox{all})}
=0.188\,(0.196),
\end{eqnarray*}
where the numbers in the parentheses are the experimental
data~\cite{Whitehouse:phd}.  These same data
are used to fix the strong coupling constants in the isobar model
of Ref.~\cite{Burkhardt:1991ms} to deduce the radiative decay widths of the $\Lambda(1405)$.

As we have seen, with the use of only one cut-off parameter and the lowest-order chiral
Lagrangian, one can reproduce fairly well all the low energy data related to the $\Lambda(1405)$,
both strong and electromagnetic.  In this work, we extend the unitary
coupled-channel chiral approach of Refs.~\cite{Oset:1997it,Oset:2001cn} to
investigate the radiative decay widths of the $\Lambda(1405)$. We also study
several related reactions to investigate the possibility of experimentally
testing the two-pole structure of the $\Lambda(1405)$ and the predictions of
the present work.

\section{The radiative decay width of the $\Lambda(1405)$}\label{sec:decay}
In the picture of the $\Lambda(1405)$ as a dynamically generated
resonance from the meson baryon interaction, the coupling of the
photon to the resonance proceeds via the coupling to its meson and
baryon components. As mentioned in the former section, gauge
invariance is preserved in this picture as shown in
Ref.~\cite{Borasoy:2005zg}. In practical terms, as shown in
Refs.~\cite{Doring:2006ub,Doring:2007rz}, it means that the
mechanisms for the $\Lambda(1405)$ decay into $\gamma\Lambda$ or
$\gamma\Sigma^0$ are given by the diagrams shown in
Fig.~\ref{figure_decayw}. The corresponding $t$-matrix elements read
\begin{eqnarray}\label{equation:effective_coupling}
-it&=& \sum_i g_{\Lambda(1405)\rightarrow i}(-e)Q_i
\left[\alpha_i\frac{D+F}{2f}+\beta_i\frac{D-F}{2f}\right]\nonumber\\
&&\times G^{\mu\nu}\sigma_\mu\epsilon_\nu\nonumber\\
&\equiv&-ig_{\Lambda(1405)\rightarrow\gamma Y}\vec{\sigma}\cdot\vec{\epsilon}
\quad\mbox{with}\quad Y=\Lambda\,\mbox{or}\,\Sigma^0
\end{eqnarray}
with $\sigma^\mu=(0,\vec{\sigma})$, where $i$ denotes any of the ten coupled channels $K^-p$, $\bar{K}^0n$,
$\pi^0\Lambda$, $\pi^0\Sigma^0$, $\eta\Lambda$, $\eta\Sigma^0$,
$\pi^+\Sigma^-$, $\pi^-\Sigma^+$, $K^+\Xi^-$, and $K^0\Xi^0$.
In Eq.~(\ref{equation:effective_coupling}) $Q_i$ is the electric
charge of the meson of channel $i$, which is $-1$, 0, 0, 0, 0, 0, 1, $-1$, 1, and 0,
respectively, for the ten coupled channels with the order given above.
The coupling constants of the $\Lambda(1405)$ to various channels, $g_{\Lambda(1405)\rightarrow i}$,
are given in Table~\ref{table:jido}. It is
to be noted that the couplings tabulated in Table~\ref{table:jido} are for
isospin channels; therefore, appropriate isospin projections are needed when
used in Eq.~(\ref{equation:effective_coupling}).  The coupling constants
$\alpha_i$ and $\beta_i$  for the 4 charged channels $K^-p$, $\pi^+\Sigma^-$,
$\pi^-\Sigma^+$, and $K^+\Xi^-$ are tabulated in Table~\ref{table_kr}.

 \begin{table}[htpb]
     \renewcommand{\arraystretch}{1.5}
 \setlength{\tabcolsep}{3mm}
\caption{\label{table_kr}SU(3) coupling constants defined in Eq.~(\ref{equation:effective_coupling}) for the channels
$K^-p$, $\pi^+\Sigma^-$, $\pi^-\Sigma^+$, and $K^+\Xi^-$. }
\begin{center}
\begin{tabular}{lcccc}
\hline\hline
  & $K^-p$ & $\pi^+\Sigma^-$ & $\pi^-\Sigma^+$& $K^+\Xi^-$ \\
  \hline  $\alpha_{MB\rightarrow\Lambda}$&$-\frac{2}{\sqrt{3}}$&$\frac{1}{\sqrt{3}}$& $
\frac{1}{\sqrt{3}}$ & $\frac{1}{\sqrt{3}}$\\
$\beta_{MB\rightarrow\Lambda}$&$\frac{1}{\sqrt{3}}$&$\frac{1}{\sqrt{3}}$&
$\frac{1}{\sqrt{3}}$ & $-\frac{2}{\sqrt{3}}$\\
$\alpha_{MB\rightarrow\Sigma^0}$&0&$1$& $-1$ & $1$\\
$\beta_{MB\rightarrow\Sigma^0}$&$1$& $-1$ & $1$&0\\
\hline\hline
\end{tabular}
\end{center}
\end{table}

The loop function $G^{\mu\nu}$ can be
easily calculated by employing gauge invariance (see e.g.
Refs.~\cite{Doring:2007rz,Close:1992ay,Oller:1998ia,Marco:1999df,Roca:2006am}).  Since the only external
momenta available in the present process are $P$ (the $\Lambda(1405)$
4-momentum) and $k$ (the photon 4-momentum), the most general amplitude can be
written as
\begin{equation}
    T=\tilde{T}G^{\mu\nu}\sigma_\mu\epsilon_\nu,
\end{equation}
with
\begin{equation}
G^{\mu\nu}=ag^{\mu\nu}+bP^\mu P^\nu+cP^\mu k^\nu+d k^\mu P^\nu+ek^\mu k^\nu.
\end{equation}
Due to the Lorentz condition $\epsilon_\nu k^\nu=0$, the two terms proportional
to $c$ and $e$ vanish. Furthermore, gauge invariance requires that
$G^{\mu\nu}k_\nu=0$, i.e.
\begin{equation}
 ak^\mu+bP^\mu(P\cdot k)+dk^\mu (P\cdot k)=0,
\end{equation}
which implies that $b=0$ and
\begin{equation}\label{eq:adrelation}
  a=-d (P\cdot k).
\end{equation}
Following these arguments, $T$ only contains the $a$ and $d$ terms.
This  can be further simplified by noting that in the rest frame of
the $\Lambda(1405)$, $\vec{P}=0$, and taking Coulomb gauge for the photon,
$\epsilon^0=0$, only the $a$ term survives. However, the $a$ term can be more
easily computed by employing the relation of Eq.~(\ref{eq:adrelation}). This is
due to the fact that on one hand, the $d$ coefficient is found convergent since, due
to dimensional reasons, it involves two powers of momentum less in the loop
functions than other individual terms, and on the other hand, there are fewer
terms which contribute to the $d$ coefficient.

Immediately, one realizes that the diagram  $(a)$ shown in
Fig.~\ref{figure_decayw} does not contribute to the $d$ term; therefore to
calculate $G^{\mu\nu}$, we only need to calculate the diagrams $(b)$ and $(c)$.
We first look at the $(b)$ diagram. The corresponding $G^{\mu\nu}$ is
explicitly written as
\begin{eqnarray}
 G^{\mu\nu}_{(b)}&=&-i\int\frac{d^4q}{(2\pi)^4}\frac{1}{q^2-m^2}\frac{1}{(q-k)^2-m^2}\\
 &&\hspace{0.5cm}\times
\frac{2M}{(P-q)^2-M^2+i\epsilon}(q-k)^\mu(2q-k)^\nu\nonumber,
\end{eqnarray}
with $m$ the meson mass and $M$ the baryon mass of the corresponding loop.
By employing the Feynman parameterization~\cite{Peskin:1995ev}
\begin{equation}
 \frac{1}{abc}=2\int^1_0dx\,\int^{1-x}_0dz\,\frac{1}{[ax+b(1-x-z)+cz]^3}
\end{equation}
and the following relation~\cite{Peskin:1995ev}
\begin{equation}
 \int d^4q'\frac{1}{(q'^2+s+i\epsilon)^3}=i\frac{\pi^2}{2}\frac{1}{s+i\epsilon},
\end{equation}
one can obtain $G^{\mu\nu}_{(b)}\sigma_\mu\epsilon_\nu$ as
\begin{eqnarray}\label{eq:dterm}
 G^{\mu\nu}_{(b)}\sigma_\mu\epsilon_\nu&=&
 \frac{2M}{(4\pi)^2}\int^1_0dx\,\int^{1-x}_0dz\,\frac{x(1-z)}{s+i\epsilon}(2P\cdot k)\vec{\sigma}\cdot\vec{\epsilon}\nonumber\\
&\equiv&G^b\vec{\sigma}\cdot\vec{\epsilon}
\end{eqnarray}
with
\begin{equation}\label{eq:sterm}
s=-m^2(1-x)+x[P^2(1-x)-M^2-2P\cdot kz].
\end{equation}
In the same way, one can calculate the $G^{\mu\nu}\sigma_\mu\epsilon_\nu$ term
corresponding to  the diagram $(c)$ by simply exchanging $M$ and $m$ in
Eq.~(\ref{eq:sterm}), and replacing $x(1-z)$ by $-xz$ in Eq.~(\ref{eq:dterm}):
\begin{eqnarray}\label{eq:dterm2}
 G^{\mu\nu}_{(c)}\sigma_\mu\epsilon_\nu&=&
 \frac{2M}{(4\pi)^2}\int^1_0dx\,\int^{1-x}_0dz\,\frac{-xz}{s'+i\epsilon}(2P\cdot k)\vec{\sigma}\cdot\vec{\epsilon}\nonumber\\
 &\equiv&G^c\vec{\sigma}\cdot\vec{\epsilon}
\end{eqnarray}
with
\begin{equation}
s'=-M^2(1-x)+x[P^2(1-x)-m^2-2P\cdot kz].
\end{equation}
It should be noted that we have neglected the magnetic term in calculating the
diagram $(c)$, which is small and vanishes in the heavy baryon limit when integrated over the loop momentum since there
are $p$-wave and $s$-wave vertices in the loop. It is
interesting to note that although the diagrams (a), (b), and (c) are all
divergent by themselves, their sum, however, is finite as can be seen from Eqs.~(\ref{eq:dterm}) and (\ref{eq:dterm2}). The
above loop functions corresponding to the diagrams (b) and (c) can be calculated
analytically, and their explicit form can be found in Ref.~\cite{Doring:2007rz},
where the systematic cancellation of the logarithmic divergences is also shown.

\begin{table*}[htpb]
\renewcommand{\arraystretch}{1.5}
\setlength{\tabcolsep}{3mm}
 \centering \caption{\label{table:decaywidth}The radiative decay widths  of the $\Lambda(1405)$
 predicted by different theoretical models, in units of keV. The values denoted by ``U$\chi$PT'' are
 the results obtained in the present study. The widths calculated for the low-energy pole and high-energy
 pole are separated by a comma.}
\begin{tabular}{c|ccccc}
\hline\hline
 Decay channel & U$\chi$PT& $\chi$QM \cite{Yu:2006sc} & BonnCQM \cite{VanCauteren:2005sm} &
NRQM & RCQM \cite{Warns:1990xi}\\\hline
 $\gamma\Lambda$ & $16.1,\,64.8$ & 168 & 912 & 143 \cite{Darewych:1983yw}, 200, 154 \cite{Kaxiras:1985zv} & 118 \\\
 $\gamma\Sigma^0$& $73.5,\,33.5$ & 103 & 233 & 91 \cite{Darewych:1983yw}, 72, 72 \cite{Kaxiras:1985zv}& 46 \\\hline\hline
Decay channel & MIT bag \cite{Kaxiras:1985zv} & chiral bag \cite{Umino:1992hi} & soliton~\cite{Schat:1994gm}&algebraic model~\cite{Bijker:2000gq}& isobar fit~\cite{Burkhardt:1991ms}\\\hline
 $\gamma\Lambda$ &60, 17 & 75 &44,40 & 116.9&$27\pm8$\\
$\gamma\Sigma^0$ &18, 2.7 & 1.9 &13,17& 155.7&$10\pm4$ or $23\pm7$\\
 \hline\hline
\end{tabular}
\end{table*}

 The radiative decay width of the $\Lambda(1405)$ is calculated according to
\begin{equation}
\Gamma=\frac{1}{\pi}|g_{\Lambda(1405)\rightarrow\gamma Y}|^2 k\frac{M_Y}{M_{\Lambda(1405)}}
\end{equation}
with $Y=\Lambda$ or $\Sigma^0$ and $k$ the center of mass 3-momentum of the
photon in the $\Lambda(1405)$ rest frame. In this work, as in
Refs.~\cite{Oset:1997it,Oset:2001cn,Lee:1998gt}, we use $f=1.15f_\pi$ with $f_\pi=93$\,MeV, $D+F=1.26$, and $D-F=0.33$.

The radiative decay widths are calculated to be
$\Gamma_{\gamma\Lambda}=64.8$\,keV and $\Gamma_{\gamma\Sigma^0}=33.5$\,keV
for the high-energy pole, and
$\Gamma_{\gamma\Lambda}=16.1$\,keV and $\Gamma_{\gamma\Sigma^0}=73.5$\,keV for the low-energy
pole.
These are tabulated in Table \ref{table:decaywidth} together with the
predictions of various other theoretical models, including the chiral quark
model ($\chi$QM)~\cite{Yu:2006sc}, the Bonn constituent quark
model~\cite{VanCauteren:2005sm}, the non-relativistic quark
models~\cite{Darewych:1983yw,Kaxiras:1985zv}, the relativistic constituent
quark model~\cite{Warns:1990xi}, the MIT bag model~\cite{Kaxiras:1985zv}, the
chiral bag model~\cite{Umino:1992hi}, the soliton model~\cite{Schat:1994gm},
the algebraic model~\cite{Bijker:2000gq}, and the isobar model
fit~\cite{Burkhardt:1991ms} to the branching ratios of the radiative decays of
the $K^-p$ atom~\cite{Whitehouse:1989yi}.

\begin{table}
\renewcommand{\arraystretch}{1.5}
\setlength{\tabcolsep}{4mm}
\centering \caption{\label{table:convol}The averaged radiative decay widths of the $\Lambda(1405)$, in units of keV.
See Eq.~(\ref{eq:gamma_ave}) for details.}

\begin{tabular}{c|c|c}
\hline\hline
  Final states & Low-energy pole & High-energy pole \\
   \hline
    $\gamma\Lambda$ & 36.6&74.6 \\
   $\gamma\Sigma^0$ &78.4&31.9\\
 \hline\hline
\end{tabular}
\end{table}

\begin{table}
\renewcommand{\arraystretch}{1.5}
\setlength{\tabcolsep}{3mm}
 \centering \caption{\label{table:reduced_coupling}
 The effective couplings defined in Eq.~(\ref{equation:reduced_coupling}).}
\begin{tabular}{ccccc}
\hline\hline
 & $K^-p$ & $\pi^+\Sigma^-$ & $\pi^-\Sigma^+$ & $K^+\Xi^-$\\
   \hline
 $g_{MB\rightarrow\gamma\Lambda}$ & $1.26$ & $0.92$ & $-0.92$ &
 $0.35$\\
 $g_{MB\rightarrow\gamma\Sigma^0}$ & $-0.33$ & $0.93$ & $0.93$ &
 $1.26$ \\
 \hline\hline
\end{tabular}
\end{table}

\begin{table}
\renewcommand{\arraystretch}{1.5}
\setlength{\tabcolsep}{3mm}
\centering \caption{\label{table:nominal}The radiative decay widths of the $\Lambda(1405)$
evaluated at the nominal $\Lambda(1405)$ mass, $M=1406.5\,\mbox{MeV}$, in units of keV. ``Low-energy pole''
and ``High-energy pole''
indicate that the coupling constants for the low-energy pole or high-energy pole from Table \ref{table:jido} are used.
}
\begin{tabular}{c|c|c}
\hline\hline
  Final states & Low-energy pole&High-energy pole\\
   \hline
    $\gamma\Lambda$ &  23.2& 33.8\\
   $\gamma\Sigma^0$ &82.4&26.2\\
 \hline\hline
\end{tabular}
\end{table}

It is interesting to note that our predictions  for
the high-energy pole seem to agree more with the predictions of other
theoretical models, i.e. they all predict  a larger $\gamma\Lambda$ decay width
than the $\gamma\Sigma^0$ decay width except the algebraic
model~\cite{Bijker:2000gq}. In addition, we note that our predictions for
the high-energy pole are approximately only half of those predicted by the
quark models~\cite{Yu:2006sc,Darewych:1983yw,Kaxiras:1985zv,Warns:1990xi},
which have long been known to fail in describing the $\Lambda(1405)$.

We have studied the effects of the finite width of the $\Lambda(1405)$ on
the calculated decay widths by convoluting
the spectral function of the resonance:
\begin{equation}\label{eq:gamma_ave}
\Gamma_\mathrm{ave.}=\frac{-\frac{1}{\pi}\int\limits^{M+\Gamma}_{M-\Gamma}d\sqrt{s}\,\Gamma_{\gamma
Y}(\sqrt{s})\,\mathrm{Im}\frac{1}{\sqrt{s}-M+i\frac{\Gamma}{2}}
\Theta(\sqrt{s}-\sqrt{s_\mathrm{th}})}{-\frac{1}{\pi}\int\limits^{M+\Gamma}_{M-\Gamma}d\sqrt{s}
\,\mathrm{Im}\frac{1}{\sqrt{s}-M+i\frac{\Gamma}{2}}
\Theta(\sqrt{s}-\sqrt{s_\mathrm{th}})},
\end{equation}
where $M$ and $\Gamma$ are the pole mass and the corresponding width for either of the two poles
of the $\Lambda(1405)$, and $s_\mathrm{th}$ is the threshold of the main decay channel $\pi\Sigma$.
The results are listed in Table \ref{table:convol}. It is easily seen that
they are qualitatively similar to those listed in Table \ref{table:decaywidth},
but the $\gamma\Lambda$ rate for the low-energy pole
has almost doubled, which might indicate relatively large uncertainties in this quantity.

It is instructive to see
the origin of these results. Since the
high-energy pole of the $\Lambda(1405)$ couples more strongly to the $\bar{K}N$
channel and the low-energy pole couples more strongly to the $\pi\Sigma$
channel (see Table \ref{table:jido}), the difference between the results for the high-energy pole and low-energy
pole can be easily understood by noting the chiral structure
of the effective coupling constants $g_{\Lambda(1405)\rightarrow\gamma\Lambda}$
and
$g_{\Lambda(1405)\rightarrow\gamma\Sigma^0}$, see Eq.~(\ref{equation:effective_coupling}).
Neglecting the dependence on the loop functions, the couplings of
$MB\rightarrow\gamma Y$ are proportional to
\begin{equation}\label{equation:reduced_coupling}
    g_{MB\rightarrow\gamma Y}\equiv Q_M\Big[\alpha_{MB\rightarrow Y}(D+F)+\beta_{MB\rightarrow Y}(D-F)\Big]
\end{equation}
where $Y$ is either $\Lambda$ or $\Sigma^0$, and $Q_M$ is the electric charge of the meson. The corresponding
couplings are tabulated in Table \ref{table:reduced_coupling}. From
this table, one immediately realizes that in the decay to the
$\gamma\Lambda$ final state, the contributions of the two intermediate channels
$\pi^+\Sigma^-$ and $\pi^-\Sigma^+$ cancel each other, though not
completely since the corresponding loop functions in these two
channels will differ by a small amount considering that they have
different but quite similar masses.

\begin{figure*}[htpb] \centering
    \includegraphics[scale=0.40]{figure2a.eps}%
    \includegraphics[scale=0.40]{figure2b.eps}
    \caption{\label{figure_loop}Comparison of the $K^-p\rightarrow
    \gamma\Lambda$ loop functions
     obtained from different schemes. See text for details.}
\end{figure*}
One can qualitatively understand the results for the partial decay widths of the two poles as follows.
The
coupling constants for these two poles differ in the relative
strength of different channels: For the high-energy pole, the coupling to
the $\bar{K}N$ intermediate channel is larger while for the low-energy pole the coupling
to the $\pi\Sigma$ channel is larger. Therefore, for the $\gamma\Lambda$ channel, using the
coupling constants for the low-energy pole instead of the high-energy pole
effectively reduces the contribution of the $K^-p$ channel while
it enhances the contribution of the $\pi^+\Sigma^-$ and $\pi^-\Sigma^+$,
but the contributions of the $\pi^+\Sigma^-$ and $\pi^-\Sigma^+$ almost
cancel each other, and thus, the net effect of using the coupling
constants for the low-energy pole instead of the high-energy pole reduces the
corresponding decay width.

On the other hand, for the decay mode to the $\gamma\Sigma^0$ final state, two
things are noteworthy. First, the contribution of the $K^-p$ channel is much
smaller compared to the contribution of the $K^-p$ channel to the decay mode
$\gamma\Lambda$. Second, the contributions of $\pi^+\Sigma^-$ and
$\pi^-\Sigma^+$ add constructively instead of destructively.
Therefore, when using the coupling constants for the low-energy pole instead of
the high-energy pole, the radiative decay width increases.

At this point, we can conclude that if different experiments actually measure
different radiative decay widths for the $\Lambda(1405)$, it can be used as
evidence for supporting the two-pole structure of the $\Lambda(1405)$.
Instead of the individual radiative decay widths, the ratio between the radiative
decay widths to the $\gamma\Lambda$ and $\gamma\Sigma^0$ final states  might
server better this purpose since in one case one has
$\Gamma_{\gamma\Lambda}/\Gamma_{\gamma\Sigma^0}>1$ and in the other case one
has $\Gamma_{\gamma\Lambda}/\Gamma_{\gamma\Sigma^0}<1$.  This controversy, if
confirmed by experiment, can only be explained by assuming that there are
actually two poles related to the nominal $\Lambda(1405)$.

At first sight, our calculated decay widths are somehow different from the
isobar model fit of H. Burkhardt and J. Lowe~\cite{Burkhardt:1991ms}. However,
one should remember that in their fit they used the nominal $\Lambda(1405)$
mass. As we can see in Table \ref{table:nominal},
when calculated at the nominal $\Lambda(1405)$ mass, with the coupling
constants of the high-energy pole, our calculated radiative decay width for the
$\gamma\Lambda$ channel is 33.8\,keV  and for the $\gamma\Sigma^0$ is 26.2\,keV.
On the other hand, if we use the coupling constants for the low-energy pole,
the results would be 23.2\,keV for the $\gamma\Lambda$ channel and 82.4\,keV
for the $\gamma\Sigma^0$ channel. It is evident that our results with the
high-energy pole coupling constants are in good agreement with the results of
the isobar model
fit: $\Gamma_{\gamma\Lambda}=27\pm8$\,keV and $\Gamma_{\gamma\Sigma^0}=23\pm
7$\,keV or $10\pm4$\,keV~\cite{Burkhardt:1991ms}, if the calculations are done
for the nominal $\Lambda(1405)$ mass. This might indicate that the $K^-p$ intermediate
channel, and thus the high-energy pole, is dominant in the process analyzed in
Ref.~\cite{Burkhardt:1991ms} to deduce the radiative decay widths.

Finally, we would like to stress the importance of the baryon-pole term of the
diagram (c) of Fig.~\ref{figure_decayw}. If instead of employing gauge invariance and calculating all
the three diagrams (a), (b), and (c) of Fig.~\ref{figure_decayw} (we call this
scheme 1), we had calculated only diagrams (a) and (b), i.e. only the contact
term and the meson-pole term (we call this scheme 2), we would have obtained different results.
The corresponding $K^-p\rightarrow \gamma\Lambda$ loop
functions are plotted in Fig.~\ref{figure_loop} as a function of the invariant mass
of the $MB$ system. The
loop functions of scheme 2 are calculated using the cutoff $\Lambda=630$\,MeV as in
Refs.~\cite{Oset:1997it,Lee:1998gt}.
It is easily seen the baryon-pole term changes the real part of the loop
function by $\sim$30\%.  As a consequence, without this term, the calculated radiative
decay width would be larger by almost 40\%.  It is also interesting to note that
the imaginary part of the contact plus meson-pole term of scheme 2 is identical
to the imaginary part of the meson-pole term of scheme 1.

\section{Exploration of possible reactions}\label{sec:reaction}

In the previous section, we have shown that the radiative decay widths of the
$\Lambda(1405)$ to $\gamma\Lambda$ and $\gamma\Sigma^0$ can be very
different depending on which of the two poles dominates.  Therefore, the
good test would be to select different reactions which give different weights to the two
poles. Such reactions can provide further evidence for the
predicted two-pole structure of the $\Lambda(1405)$.  A first evidence for the
two-pole structure of the $\Lambda(1405)$ has been provided in
Ref.~\cite{Magas:2005vu}. By investigating the invariant mass distribution of
the $\pi^0\Sigma^0$ final state in the $K^-p\rightarrow\pi^0\pi^0\Sigma^0$
reaction, it was shown that this reaction gives more weight to the high-energy
pole of the $\Lambda(1405)$ in contrast to the reaction $\pi^-p\rightarrow
K^0\pi\Sigma$, where the low-energy pole is believed to be dominant. This
$\pi^-p\rightarrow K^0\pi\Sigma$ reaction has been studied in
Ref.~\cite{Hyodo:2003jw}. The authors found that the pure chiral mechanism
alone cannot reproduce the experimental invariant mass distributions. However,
by explicitly taking into account the contribution of the $N^*(1710)$, which
gives more weight to the $\pi\Sigma$ channel, and thus more weight to the low-energy
pole, they found that the experimental data can be reasonably described.  In
the following, we study the corresponding electromagnetic reactions
$K^-p\rightarrow \pi^0\gamma \Lambda(\Sigma^0)$ and $\pi^- p\rightarrow
K^0\gamma \Lambda(\Sigma^0)$ in more detail.
\begin{figure*}[htpb]
 \centering
\includegraphics[scale=0.7]{figure3.eps}
\caption{\label{figure_kp}The diagrams contributing to the reaction $K^-p\rightarrow \pi^0\gamma\Lambda(\Sigma^0)$.}
\end{figure*}
\begin{figure*}[htpb]
 \centering
 \includegraphics[scale=0.7]{figure4.eps
 \caption{\label{figure:tmatrix}The strong amplitude $T$.}
\end{figure*}
\begin{figure*}[htpb]
 \centering
\includegraphics[scale=0.7]{figure5.eps}
\caption{\label{figure:gmatrix}The electromagnetic amplitude $A$.}
\end{figure*}

\subsection{The $K^-p\rightarrow \pi^0\gamma\Lambda(\Sigma^0)$ reaction}

In Ref.~\cite{Magas:2005vu}, it was found that the reaction $K^-p\rightarrow
\pi^0\pi^0\Sigma^0$ is dominated by the so-called nucleon-pole mechanism. By
analogy, the $K^-p\rightarrow \pi^0\gamma \Lambda(\Sigma^0)$ reaction should
also proceed through the same mechanism, which is explicitly shown in
Figs.~\ref{figure_kp}, \ref{figure:tmatrix}, and \ref{figure:gmatrix}.  The corresponding $t$-matrix reads
\begin{equation}
-it=-iA\vec{\sigma}\cdot\vec{\epsilon}\,\vec{\sigma}\cdot\vec{v}-iB\vec{\epsilon}\cdot\vec{p}_a\,\vec{\sigma}\cdot
(\vec{p}_a-\vec{p}_2)\,\vec{\sigma}\cdot\vec{v},
\end{equation}
where $\vec{v}=\vec{p}_1(1+\frac{p_1^0}{2M_N})+\frac{p_1^0}{M_N}\vec{p}_a$, $A$ and $B$ are
\begin{eqnarray}\label{eq:tmatrixA}
A&=&\frac{D+F}{2f_\pi}\frac{M_N}{E_N(\vec{p}_a+\vec{p}_1)}\frac{1}{E_N-p_1^0-E_N(\vec{p}_a+\vec{p}_1)}\nonumber\\
&&\times
\Bigg[\sum_j T_{k^-p\rightarrow j}(M_I)(G^b(M_I)+G^c(M_I))\nonumber\\
&&\hspace{1.2cm}\times(-e)Q_j\left(\alpha_j\frac{D+F}{2f}+\beta_j\frac{D-F}{2f}\right)\nonumber\\
&&\hspace{0.6cm}
+(-e)Q_1\left(\alpha_1\frac{D+F}{2f}+\beta_1\frac{D-F}{2f}\right)\Bigg],
\end{eqnarray}
\begin{eqnarray}
B&=&\frac{D+F}{2f_\pi}\frac{M_N}{E_N(\vec{p}_a+\vec{p}_1)}\frac{1}{E_N-p_1^0-E_N(\vec{p}_a+\vec{p}_1)}\nonumber\\
&&\times\frac{-2eQ_1}{(p_a-p_2)^2-m_a^2}\left[\alpha_1\frac{D+F}{2f}+\beta_1\frac{D-F}{2f}\right],
\end{eqnarray}
with $M_N$ the nucleon mass, $E_N$ the nucleon energy, and $M_I^2=(p_2+p_3)^2$. The last term of Eq.~(\ref{eq:tmatrixA}) accounts for the first tree
level diagram of Fig.~\ref{figure_kp}, while the other part of the $A$ coefficient proportional to
$T_{K^-p\rightarrow j}$ accounts for the third diagram (loop diagram) of Fig.~\ref{figure_kp}. The term $B$
corresponds to the second tree level diagram of Fig.~\ref{figure_kp}.
In Eq.~(\ref{eq:tmatrixA}), the $T_{k^-p\rightarrow j}$, with $j$ referring to the
ten coupled channels, are the
strong amplitudes of Ref.~\cite{Oset:2001cn}, which is diagrammatically shown in Fig.~\ref{figure:tmatrix}. The loop functions $G^b$ and $G^c$ are those of Eqs.~(\ref{eq:dterm}) and (\ref{eq:dterm2}).

The invariant mass distribution is then calculated by
\begin{eqnarray}\label{eq:inv:infra}
\frac{d\sigma}{dM_I}&=&\frac{1}{4}\frac{M_N M_Y}{\lambda^{1/2}(s,M_N^2,m_K^2)}\frac{M_I}{\sqrt{s}}\frac{1}{(2\pi)^4}\nonumber\\
&&\times\int^1_{-1}d\cos\theta_1
\int^{E_\mathrm{max}}_{E_\mathrm{min}} dE_2\int^{2\pi}_0d\phi_{12}\bar{\sum}\sum|t|^2\nonumber\\
&&\hspace{1cm}\times\theta(1-\cos^2(\theta_{12}))
\end{eqnarray}
where $\sqrt{s}$ is the center of mass energy of $K^- p$, $\theta_1$ is the angle between $\vec{p}_a$ and $\vec{p}_1$, $\theta_{12}$ is the angle between
$\vec{p}_1$ and $\vec{p}_2$, fixed by kinematics, while $\phi_{12}$ is the azimuthal angle of $\vec{p}_2$
with respect to a frame where $\vec{p}_1$ is chosen in the $z$ direction. In addition,
$E_\mathrm{min}=0$,
$E_\mathrm{max}=\frac{s-(m_1+m_3)^2}{2\sqrt{s}}$, and
\begin{equation}
\cos(\theta_{12})=\frac{1}{2|\vec{p}_1||\vec{p}_2|}\left\{
(\sqrt{s}-E_1-E_2)^2-m^2_3-\vec{p}_1^2-\vec{p}_2^2\right\},
\end{equation}
\begin{eqnarray}
\bar{\sum}\sum|t|^2&=&|v|^2
 \Bigg\{\{2|A|^2+\left(|\vec{p}_a|^2-\frac{(\vec{p}_a\cdot\vec{p}_2)^2}{|\vec{p}_2|^2}\right)\nonumber\\
&&\times\left[(A^*B+AB^*)+
|B|^2(\vec{p}_a-\vec{p}_2)^2\right]\Bigg\}.\nonumber\\
\end{eqnarray}
The invariant mass distributions for the reactions $K^-p\rightarrow \pi^0\gamma\Lambda$ and
$K^-p\rightarrow \pi^0\gamma\Sigma^0$ for a kaon of laboratory momentum 687\,MeV
are shown in Fig.~\ref{figure_kp2}. It is seen
that both the invariant mass distributions exhibit a peak at $\sim$1420\,MeV,
 and therefore manifesting the high-energy pole of the $\Lambda(1405)$.  The invariant
mass distribution is also different from a Breit-Wigner shape, particularly
that of the $\gamma\Lambda$ channel, which is due to the background terms (the
tree-level diagrams in Fig.~\ref{figure_kp}).

It is interesting to recall that in Refs.~\cite{Oset:1997it,Oset:2001cn}, the
two poles,  one at 1390\,MeV with a width of 132\,MeV and the other at
1426\,MeV with a width of 32\,MeV, are generated through the interaction of the ten coupled
channels. The low-energy pole couples more strongly to the $\pi\Sigma$ channel
while the high-energy pole couples more strongly to the $\bar{K}N$ channel.  It
was argued in Ref.~\cite{Jido:2003cb} that reactions favoring different
channels would lead to different invariant mass distributions giving more
weight to one pole or the other.  It should be noted that in
Ref.~\cite{Oset:1997it}, the experimental invariant mass distribution was
produced by the following formula
\begin{equation}\label{eq:inv}
\frac{d\sigma}{dm_\alpha}=C|T_{\pi\Sigma\rightarrow\pi\Sigma}|^2P_\mathrm{CM},
\end{equation}
and thus giving more weight to the low-energy pole and resulting in a peak at
$\sim$1400\,MeV. However, in the presence of two resonances, the different
$T_{ij}$ amplitudes do not peak at the same place, and particularly, $T_{\bar{K}N\rightarrow\pi\Sigma}$
peaks at higher energies than $T_{\pi\Sigma\rightarrow\pi\Sigma}$~\cite{Jido:2003cb}.
In such a case, Eq.~(\ref{eq:inv}) should be replaced ~\cite{Jido:2003cb} by
\begin{equation}
    \frac{d\sigma}{dm_\alpha}=|\sum C_i T_{i\rightarrow\pi\Sigma}|^2P_\mathrm{CM}.
\end{equation}
Hence, if the reaction mechanism does not
completely forbid a $\bar{K}N$ channel, then the peak should always be shifted
towards higher energy.  Thus, it is not surprising that the invariant mass distributions of all the three
reactions~\cite{Nacher:1998mi,Nacher:1999ni,Magas:2005vu} studied previously
including the present one exhibit a peak around $\sim$1420\,MeV.
\begin{figure}[tp]
 \centering
\includegraphics[scale=0.42]{figure6.eps}
\caption{\label{figure_kp2}The invariant mass distribution of $K^-p\rightarrow \pi^0\gamma
\Lambda(\gamma\Sigma^0)$ as a function of the invariant mass of the final
$\gamma\Lambda$($\gamma\Sigma^0$) system.}
\end{figure}
\begin{figure}
 \centering
    \includegraphics[scale=0.42]{figure7.eps}
\caption{The modulus squared of the strong amplitudes obtained from the model of
Ref.~\cite{Oset:2001cn}.}
\label{fig:amplitude}
\end{figure}

It is worth pointing out an interesting difference between the reactions studied in
this work and the other reactions~\cite{Nacher:1998mi,Nacher:1999ni,Magas:2005vu}. In the reaction
$K^-p\rightarrow\pi^0\gamma\Lambda(\Sigma^0)$ and the reaction
$\pi^-p\rightarrow K^0\gamma\Lambda(\Sigma^0)$, which will be studied below, the
$K^-p\rightarrow K^-p$ channel appears as an intermediate channel. Since the
magnitude of the $t$-matrix of this channel is much larger than those of the other channels,
and since
this channel manifests the high-energy pole (see Fig.~\ref{fig:amplitude}), one can always expect a peak at
$\sim1420$\,MeV in the invariant mass distribution of the final states unless
some reaction mechanisms largely suppress this channel. On the other hand, in
the $\pi\Sigma$ final states studied in
Refs.~\cite{Nacher:1998mi,Nacher:1999ni,Magas:2005vu}, the $T_{\bar{K}N\rightarrow\bar{K}N}$
does not
contribute and because the $\bar{K}N\rightarrow \pi\Sigma$ and
$\pi\Sigma\rightarrow\pi\Sigma$ amplitudes have
similar strength (in fact the modulus of the
$K^-p\rightarrow \pi\Sigma$ amplitude
is still approximately two times larger than that of the $\pi\Sigma\rightarrow\pi\Sigma$ amplitude
at their respective peak positions), the invariant mass distributions
will be a superposition of the two peaks, and, depending on the reaction mechanism,
the final distribution will peak at one or another energy.  This situation is somewhat similar to the two-pole
structure of the $K_1(1270)$~\cite{Geng:2006yb}. There, it was found that due to the
dominance of the $\rho K\rightarrow \rho K$ amplitude over the other amplitudes
leading to the $\rho K$ final states, a prominent peak at $\sim 1280\,\mbox{MeV}$ would be
preferred in the invariant mass distribution of the $K\pi\pi$ system leading to
$\rho K$ final states.

\begin{figure*}[htpb]
 \centering
\includegraphics[scale=0.7]{figure8.eps}%

\caption{\label{figure_nstar1}The diagrams contributing to the reaction $\pi^-p\rightarrow K^0\gamma\Lambda(\Sigma^0)$.}
\end{figure*}
\subsection{The $\pi^- p\rightarrow K^0\gamma\Lambda(\Sigma^0)$ reaction}

In Ref.~\cite{Hyodo:2003jw}, it was shown that the reaction $\pi^-p\rightarrow K^0\pi\Sigma$ can
be reasonably described in terms of $t$-channel and $s$-channel resonance exchanges.
The corresponding electromagnetic reaction $\pi^-p\rightarrow K^0\gamma\Lambda(\Sigma^0)$, in principle, should
also proceed through similar mechanisms. Nevertheless,
since we only want to make an exploratory study of this reaction, we neglect the
mechanisms of $t$-channel meson exchange (and associated contact $MMBBB$ terms),
referred to as chiral terms in Ref.~\cite{Hyodo:2003jw},  and concentrate on the
$s$-wave $N^*(1710)$ resonance contribution, which was found to be largely dominant in Ref.~\cite{Hyodo:2003jw}.

The $t$-matrix element corresponding to the resonance mechanism shown in Fig.~\ref{figure_nstar1}
reads
\begin{eqnarray}
-it&=&(-it_{\pi^-p\rightarrow N^*})\frac{i}{\sqrt{s}-M_\mathrm{R}+i\frac{\Gamma}{2}}\nonumber\\
&&\hspace{1cm}\times\sum_i(-it_{N^*\rightarrow K^0i})
(-it_{i\rightarrow \gamma\Lambda(\Sigma^0)})
\end{eqnarray}
with
\begin{equation}
-it_{\pi^-p\rightarrow N^*}=\frac{A}{f_\pi}\vec{\sigma}\cdot\vec{p}_a,
\end{equation}
\begin{equation}\label{eq:suppression}
-it_{N^*\rightarrow K^0i}=i\frac{\tilde{B}}{f^2}C_{i}(\omega_{i}-\omega_{K^0}),
\end{equation}
\begin{eqnarray}
-it_{i\rightarrow\gamma\Lambda(\Sigma^0)}&=&
\sum_j\left(G_i(M_I)T_{i\rightarrow j}(M_I)+\delta_{ij}\right)(G^b_{j}+G^c_j) \vec{\sigma}\cdot\vec{\epsilon}\nonumber\\
&&\times
\left[
-ieQ_j\left(\alpha_j\frac{D+F}{2f}+\beta_j\frac{D-F}{2f}\right)\right],
\end{eqnarray}
where $i$, $j$ can be any of the ten coupled channels. The couplings constants $C_i$
can be found in Table II of Ref.~\cite{Hyodo:2003jw}. The loop function $G_i$ is
that of one meson and one baryon, which is calculated in the
dimensional regularization scheme and with the same
subtraction constants as in Ref.~\cite{Oset:2001cn} . The meson energies $\omega_i$ and
$\omega_{K^0}$ are calculated by
\begin{equation}
    \omega_{K^0}=\frac{s+m^2_K-M^2_I}{2\sqrt{s}},
\end{equation}
\begin{equation}
    \omega_i=\frac{M^2_I+m^2_i-M^2_i}{2M_I},
\end{equation}
with $\sqrt{s}$ the invariant mass of $\pi^- p$, $m_i$ and $M_i$ the meson and baryon masses of channel $i$, and $M_I$ the
$\gamma\Lambda(\Sigma^0)$ invariant mass.

\begin{figure}[tpb]
 \centering
\includegraphics[scale=0.42]{figure9.eps}
\caption{\label{figure_nstar2}The invariant mass distribution of $\pi^-p\rightarrow K^0\gamma
\Lambda(\gamma\Sigma^0)$ as a function of the invariant mass of the final $\gamma\Lambda$($\gamma\Sigma^0$) system.}
\end{figure}
In our calculation, the
parameter set II of Ref.~\cite{Hyodo:2003jw} is used, i.e. $M_R=1740$\,MeV,
$|A|=0.1344$, $|\tilde{B}|=0.842$, $\Gamma(\sqrt{s}=2020\mbox{ MeV})=776$\,MeV.
The invariant mass distributions are calculated by
\begin{equation}
\frac{d\sigma}{dM_I}=\frac{M_N M_Y}{\lambda^{1/2}(s,M^2_N,m^2_\pi)}\frac{1}{(2\pi)^3}\frac{1}{\sqrt{s}}p_1\tilde{p}_2
\bar{\sum}\sum|t|^2
\end{equation}
with
\begin{equation}
p_1=\frac{\lambda^{1/2}(s,M_I^2,m_1^2)}{2\sqrt{s}},\quad \tilde{p}_2=\frac{\lambda^{1/2}(M_I^2,m_2^2,m_3^2)}{2M_I},
\end{equation}
and are shown in Fig.~\ref{figure_nstar2} for a pion of laboratory momentum 1690\,MeV.
At first sight, two things are
surprising. First, the $\pi^-p\rightarrow K^0\gamma\Lambda$ reaction still exhibits a
peak around $\sim$1420\,MeV. Second, the magnitude of the $\pi^-p\rightarrow
K^0\gamma\Lambda$ is still larger than that of $\pi^-p\rightarrow
K^0\gamma\Sigma^0$. This is due to the following reasons: As we have
noticed in the previous section, the $\pi^+\Sigma^-\rightarrow
\gamma\Lambda$ term and the $\pi^-\Sigma^+\rightarrow \gamma\Lambda$ term
nearly cancel each other. Therefore, it is natural that the
$\pi^-p\rightarrow K^0\gamma\Lambda$ reaction still manifests the high-energy pole of the
$\Lambda(1405)$ since in this reaction the $K^-p\rightarrow \gamma\Lambda$
intermediate channel contributes most.  While in the $\pi^-p\rightarrow K^0\gamma\Sigma^0$ reaction,
the contribution of $K^-p\rightarrow \gamma\Sigma^0$ itself is small and is
further suppressed by the $\omega_{K^-}-\omega_{K^0}$ factor of Eq.~(\ref{eq:suppression}). On the other
hand, the $\pi^+\Sigma^-\rightarrow\gamma\Sigma^0$ and
$\pi^-\Sigma^+\rightarrow\gamma\Sigma^0$ terms  add constructively and both give
more weight to the low-energy pole of the $\Lambda(1405)$. Therefore, the net
result is a broad peak around $\sim$1390\,MeV, in agreement with the finding of
Ref.~\cite{Hyodo:2003jw}. The larger magnitude of $\pi^-p\rightarrow
K^0\gamma\Lambda$ is due to the fact that the strong amplitude $K^-p\rightarrow
K^-p$ is much larger than the other $i\rightarrow j$ amplitudes, as we have discussed previously.

\section{Summary and conclusions}\label{sec:summary}
Using the unitary extension of the chiral perturbation  theory U$\chi$PT, we
have calculated the radiative decay widths of the $\Lambda(1405)$. Since there
are two poles in the U$\chi$PT
models corresponding to the nominal $\Lambda(1405)$, our calculations, using the model of Refs.~\cite{Oset:1997it,Oset:2001cn}, result in two different
radiative decay widths. For the high-energy pole, our calculated widths,
$\Gamma_{\gamma\Lambda}$=64.8\,keV and $\Gamma_{\gamma\Sigma^0}$=33.5\,keV, are
in qualitative agreement with the predictions of the isobar model fit, in
particular, when evaluated at the nominal $\Lambda(1405)$ mass where the agreement is
very good, but they are in sharp contrast
with those of the quark models and the bag models.  The disagreement with the
quark model predictions adds to the list of other magnitudes that
the quark models also fail to reproduce. For instance, the $\Lambda(1405)$ and the
$\Lambda(1520)$ are degenerate in the model of Ref.~\cite{Isgur:1978xj}.

We also evaluated the radiative decay width for the low-energy pole, and we obtain a totally different
result with $\Gamma_{\gamma\Lambda}=16.1$\,keV and
$\Gamma_{\gamma\Sigma^0}=73.5$\,keV. These are completely different from all
the existing model predictions. All the other theoretical models predict a larger
$\gamma\Lambda$ decay width while a smaller $\gamma\Sigma^0$ decay width except
the  algebraic model~\cite{Bijker:2000gq}.

To find a possible reaction which might give different weights to the two
poles of the $\Lambda(1405)$, we have studied the reactions
$K^-p\rightarrow\pi^0\gamma\Lambda(\Sigma^0)$ and $\pi^-p\rightarrow
K^0\gamma\Lambda(\Sigma^0)$.  These two reactions share a lot of similarities
with the corresponding hadronic reactions, $K^-p\rightarrow\pi^0\pi^0\Sigma^0$
and $\pi^-p\rightarrow K^0\pi\Sigma$, which have been previously studied in
Refs.~\cite{Magas:2005vu,Hyodo:2003jw} and found to yield reasonable agreement
with the data. Our studies show that both these reactions yield a larger
$\gamma\Lambda$ cross section and a smaller $\gamma\Sigma^0$ cross section.
This reflects a non-trivial feature of the U$\chi$PT model: the magnitude of the
$K^-p\rightarrow K^-p$ amplitude is much larger than that of the other amplitudes. On
the other hand, there are subtle differences between the two reactions studied,
$K^-p\rightarrow\pi^0\gamma\Lambda(\Sigma^0)$ and $\pi^- p\rightarrow K^0\gamma\Lambda(\Sigma^0)$.
While
the first reaction gives more weight to the high-energy pole in both channels,
the second reaction gives more weight to the high-energy pole in the
$\gamma\Lambda$ channel and  to the
low-energy pole in the $\gamma\Sigma^0$ channel. This is
reflected by exhibiting a narrower peak at $\sim1420$\,MeV in
the former channel and a broader peak at $\sim1390$\,MeV in the latter channel.
The total cross sections for the $K^-p$ reaction
at $p_K(\mbox{lab})=687$\,MeV  are 1.78\,$\mu b$
($\gamma\Lambda)$ and 0.41\,$\mu b$ ($\gamma\Sigma^0$), which are integrated [see Eq.~(\ref{eq:inv:infra})] with the lower
limit $M_I=1300\,$MeV to avoid infrared divergence. The cross sections
for the $\pi^-p$ reaction
at $p_\pi(\mbox{lab})=1690$\,MeV turn out to be $3.90\times10^{-2}$\,$\mu b$
($\gamma\Lambda$) and $1.58\times 10^{-2}$\,$\mu b$ ($\gamma\Sigma^0$).

Therefore, an experimental measurement of the radiative decay widths of the
$\Lambda(1405)$ in the related reactions, such as
$K^-p\rightarrow\pi^0\gamma\Lambda(\Sigma^0)$ and $\pi^-p\rightarrow K^0\gamma\Lambda(\Sigma^0)$, not only
would lend further support to
the predicted two-pole structure of the $\Lambda(1405)$ but also to the underlying
chiral unitary approach, which so far
has provided a systematic and consistent description of the $\Lambda(1405)$ and low-energy
reactions involving it.

\section{Acknowledgments}
L. S. Geng acknowledges useful communications with Dr. T. Hyodo and financial support
from the Ministerio de Educacion y Ciencia in the Program of estancias de doctores y
tecnologos extranjeros. This work is
partly supported by DGICYT contract number Fis2006-03438 and the Generalitat
Valenciana.
This research is part of the EU Integrated Infrastructure Initiative Hadron
Physics Project under contract number RII3-CT-2004-506078.

redpajama_set_name: RedPajamaArXiv


Secretary General of the Government Toni Grebla said that the prime minister will send president Klaus Iohannis the same proposals for the Ministries of Transport and Development, namely Lia Olguta Vasilescu and Mircea Draghici. Toni Grebla made the statement for Digi 24.
"This will certainly be the decision and it will be taken today," said Secretary General of the Government, Toni Grebla.
He also told Hotnews that President Klaus Iohannis's explanations for the rejection of the ministers proposed for Transport and Development are "unrelated to legal and constitutional provisions".
"Unfortunately, the president did not point to the specific issues related to the provisions of Article 105 of the Constitution, nor from Article 2 of Law 90/2001. The answer is a political one and it is unrelated to legal and constitutional provisions," Grebla told Hotnews.
President Klaus Iohannis sent two letters to Prime Minister Dancila on Thursday explaining why he rejected his proposals to appoint new ministers for Transport and Development.
In the first letter, the president explains why he did not appoint Ilan Laufer and Olguta Vasilescu to Development, respectively Transport, in the first phase of the government reshuffle. About Laufer the head of state says that the legal conditions are not met, and that Vasilescu does not have the necessary expertise. In the second letter, the president claims that he did not appoint Mircea Draghici and Olguta Vasilescu in Transport, respectively Development, because there is no mention of the fulfillment of the conditions of legality from the documentation submitted.


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Today was our first day of the Thursday Morning Four-Play Challenge for the Summer Season. The usual volunteers showed up to clean up the courts and prepare them for play. We had Twenty-Four (24) enthusiastic shufflers show up from CMS, Deland and Orange City to meet the challenge. We played four games of 16 frames or 75 points and recorded the wins at the end of each match. When the dust had cleared Dennis, Charlie and Randy had won all four of their games. Congratulations. Hope to see you all back here next week for the next challenge.


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    public class ToUpperConverter : IValueConverter
    {
        public object Convert(object value, Type targetType, object parameter, CultureInfo culture)
        {
            if (value is string)
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                return ((string) value).ToUpper();
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    }
}

redpajama_set_name: RedPajamaGithub


At Fermor, we provide a safe and stimulating environment. The teachers and TA's observe and assess learning to inform next steps. We see every child as an individual and plan exciting and playful activities based on the children's interests and development.
Children in the EYFS learn by playing and exploring, being active, and through creative and critical thinking which takes place both indoors and outside. This is referred to as the Characteristics of Effective Learning.
Children in reception attend Forest School weekly. This takes place in our attractive woodland area. Experiences include outdoor woodland games, craft in the natural environment and cooking over the fire. Play is recognised as an important part of Forest School and activities are based on the children's interest and unique way of learning.
At Fermor we pride ourselves on our partnership with parents. We use Tapestry, an online learning journal, to share the children's development as well as communicate important information and dates with parents. This is a two way communication, with parents adding their own observations of their child, which is shared with the class. The children love to share their experiences whilst developing their confidence and language skills.
At Fermor we feel that the transition from pre school to nursery is a big step for children (and parents). Therefore we provide supportive opportunities for the children to visit their new classroom and get to know the team through stay and play sessions, story times and nursery visits in term 6. Before children start in Reception, a home visit is offered to new parents, giving the opportunity to talk informally with the Early Years Foundation Stage staff.
We promote British Values through Learning and Play. We support children's Personal Social and Emotional development (PSED) by developing their self confidence and self awareness; giving opportunities to the children to make choices about what they choose to learn and the resources they will need. We encourage the children to manage their own feelings and behaviour. The children put together a list of expectations and rules and this is reflected on regularly. Each class has a class value. Hedgehogs is Joy and Owls is Hope.


Returning to the Philippines after three years, Boyzone performed at the Mall of Asia Arena on August 26, Sunday, as part of their 25th Anniversary and Farewell tour.
The Irish boy band – Ronan Keating, Keith Duffy, Mikey Graham and Shane Lynch – performed their most loved hits like Love Me For A Reason, Father and Son, Picture of You, Love You Anyway, Love is a Hurricane and more. They also paid tribute to band member Stephen Gately who died in 2009 with the song Gave It All Away and Everyday I Love You.
Boyzone's 25th Anniversary and Farewell Tour is presented by Ovation Productions.
This is the final chance for their millions of Filipino fans to watch them perform together.