text:
Wells, Pumps, &C
STEAM BORING MACHINE FOR QUARRIES, —amp;c.—mdash;The annexed engravings are views of STEAM BORING MACHINE FOR QUARRIES, —amp;c.—mdash;The annexed engravings are views of steam machinery for boring by M. Cave, of Paris, a celebrated French engineer, and which has been illustrated in the " London Artisan." For the great majority ot mining, quarrying, and tunnelling operations, boring and blasting is employed, and it is for this object that M. Cave's machinery is designed. It consists of a cylinder and piston actuated by steam, compressed air, or by the vacuum system, the cutting tools being attached to the piston-rod, and acting by percussion. It thus resembles a Nasmyth's steam hammer; and a similar means is employed to destroy the momentum of the piston, by enclosing a portion of steam or air, which acts as a cush ion at each end of the cylinder. To carry out this purpose, the inlet aria exhaust passages are kept quite distinct, as will be seen on re ferring to the drawings. Figure 1 is an elevation of the machine in section through the inlet passages ; figure 2 is an elevation of the cylinder in section through the outlet passages; figured is a front eleva tion, showing the passages; and figure 4 is a plan in section through the passages. J is the cylinder, containing the piston, K, to the rod of which is attached a cross-head, N, to which is also fixed the chisel, M. The cross-head arid chisel are guided by the guide-rods, 0 0, which are fixed in a plate dovetailed into the cylinder cover, in such a manner, that it can be freely turned round (with the piston). by means of the handles, P Q, and thus enable the chisel to take a fresh cut at every stroke, without which it would jam. The annexed sketches show the shape of the chisel and its cutting edge. The admission and emission of the com pressed air or steam is regulated by a four-way cock, R, supplied by a pipe, T, as shown in figure 1. The air is admitted through the inlet passage, a,, on the top of the piston, which will rapidly descend, until it passes the outlet, a', figure 2, when, the further escape of air being prevented, the piston is stopped by the air-cushion. On the up-stroke, the cock having been turned, the compressed air enters by the passage, b, and escapes by the passage, b'. It will be observed that the plug of the cock is divided transversely by a dia phragm, shown in fig. 4, to keep the passages distinct, c and d answering to the two inlet passages, and t and f to the two outlets. The air which escapes by the cylinder is led, by the pipe, t, to near the point of the chisel, and will have the effect of blowing away the small chips loosened by the chisel. The machine is shown in "the engraving as working vertically; but it could obviously be applied to driving a level, by placing it hori zontally and mounting it on a carriage. If it be desired to bore a hole of larger dia meter than the width of a chisel, the cutter can be fixed at any desired distance from the centre of the piston-rod, the revolution of which will cause the cutter to describe a cir cle of corresponding diameter. For sinking shafts, a number of cylinders might be employed simultaneously, working a sufficient number of chisels to extend round the shaft; and the same arrangement applied horizontally would serve to drive a level.—mdash; In vertical boring the chisels have to be regu larly withdrawn, in order to permit ot the extraction of the debris; but we do not find that the author has provided any special means for effecting this object. He has suggested that the electro-magnetic power may be applied to work this machine ry; but air appears to offer the most tangible advantages. It can be conducted a great dis tance without suffering condensation, as steam does; and it would materially improve the atmosphere ot the mine, by blowing in fresh air, or, if worked on the vacuum system, it would be equally advantageous in coal mines, by serving to draw off the fire-damp.
This article was originally published with the title "Wells, Pumps, &C" in Scientific American 8, 22, 176 (February 1853)
doi:10.1038/scientificamerican02121853-176a
More Airports to Use Greener 'Glide' Approach to Landing
Minho Kim and E&E News
How Do We Really Age?
In the store
Scientific American Volume 8, Issue 22


This is a group for finding other people with the same interest in running/jogging. Doesn't matter if you've completed your tenth marathon or you are just starting out and can barely complete one mile. We welcome all levels.
Hopefully you will find someone to train with you and keep you motivated!


text:
Tag Archives: Budapest Quartet
MEET THE ROYAL GARDEN TRIO
The Royal Garden Trio's new CD (2010)
I have to come out with it: the seventy-five minute span of a compact disc is often too much for me. So when I loaded the first of three discs by the Royal Garden Trio into the car player, I expected the outcome to be the same: restlessness halfway through. No, the Beloved and I (she's a stern critic herself) played the three discs nonstop during a six-hour drive.
They're that good.
On these CDs, the RGT is made up of Mike Karoub (cello and string bass); Tom Bogardus (tenor guitar and clarinet), Brian Delaney (acoustic and electric 6-string guitars). And they have eminent guest stars: Jon-Erik Kellso (trumpet); James Dapogny (piano); Bess Bonnier (piano, heard on JITTERBUG WALTZ below); Chris Smith (sousaphone), Louis Caponecchia (ukulele / vocal); Jo Serrapere, Paul King, Melissa Brady (vocals); Gian Paulo (string bass), Rod McDonald (guitar), Donn Deniston (drums).
What makes the Royal Garden Trio so delightful is their own restrained eloquence. The world is full of enthusiastic Hot Club spinoffs — very capable musicians, inspired by Django and Stephane. But often the result is "note for note," which is amazing technically but less so aesthetically, or an overabundance . . . many notes, many choruses, fast tempos, dalling string virtuosity. One part of the brain admires; the other portion asks (in Lester Young's words) to be told a story.
The members of the RGT have beautiful stories to tell. They are virtuosic as well, but they know that too much is not a good thing. So their solos are thoughtful speech, not diatribes; their notes ring and resound in the air. Each player creates compelling melodies, and they work together like a swing version of the Budapest Quartet.
Since I often find the heirs to Grappelli are given to excessive sweetness and high drama, I am thrilled by Karoub's cello: earnest, dark yet lithe. Mike's conception is never overblown, but his solos can be majestic. Delaney's guitar is part Lang, part Lonnie Johnson. Bogardus romps on his guitar and his clarinet playing is easy, fervent, balancing Dodds and klezmer. And the trio works together to create something beautiful, varied, and cheering. Their performances are marvelous vignettes, the guitarists switching lead and rhythm, Bogardus playing a chorus on clarinet; Karoub bowing and then plucking in a propulsive manner (across bar lines) that recalls Steve Brown.
And they swing — without even trying hard.
Although much of the repertoire is familiar, the trio's approach lifts it up: I never found myself saying, "Oh, another ST. LOUIS BLUES," but was excited by what this band can do. And the CDs offer some less-played material as well: Ellington's SATURDAY NIGHT FUNCTION, LOUISIANA FAIRY TALE (for the home-improvement minded among us, but this time with the verse), THERE'LL COME A TIME, RAGGIN' THE SCALE, I'M FOREVER BLOWING BUBBLES, GO INTO YOUR DANCE, a hidden track of APRIL KISSES, and some winding originals that sound like theme music for mid-Thirties screwball comedy films.
The RGT's debut CD, 2002
But you can hear and see the Trio for yourself courtesy of YouTube:
HOW DEEP IS THE OCEAN? (which Mike Karoub informs me was Moe Howard's favorite song, a valuable fact):
JITTERBUG WALTZ (with the legendary Bess Bonnier on piano):
The RGT's second CD, 2005
To find out more, visit the Trio's website: http://www.theroyalgardentrio.com/sched.html. And if you feel moved to purchase all three discs (I recommend this) ask for the JAZZ LIVES discount. These players (and their nimble friends) will bring joy, in or out of the car.
SWING OUT WITH PAYPAL! ALL MONEY COLLECTED GOES TO THE MUSICIANS:
https://.paypal.com/cgi-bin/webscr?cmd=_s-xclick&hosted_button_id=VBURVAWDMWQASwww
Posted in "Thanks A Million", Irreplaceable, Jazz Titans, Pay Attention!, Swing You Cats!, The Heroes Among Us, The Real Thing, The Things We Love
Tagged Bess Bonnier, blue notes, Brian Delaney, Budapest Quartet, Chris Smith, Django Reinhardt, Donn Deniston, Eddie Lang, Gian Paulo, Gypsy Swing, Hot Club, James Dapogny, Jo Serrapere, Johnny Dodds, Jon-Erik Kellso, klezmer, Lester Young, Lonnie Johnson, Louis Caponecchia, Melissa Brady, Mike Karoub, Moe Howard, Paul King, Quintette of the Hot Club of France, Rob Bourassa, Rod McDonald, Royal Garden Trio, Stephane Grappelly, Steve Brown, swing, Tom Bogardus
DAN BLOCK'S VIVID IMAGINATIONS
Dan Block is a peerless reed player, arranger, composer, bandleader. A new CD captures his many imaginations whole. The picture (by Dan's daughter Emma) adorns the cover of his Ellington tribute, FROM HIS WORLD TO MINE.
Tributes to Ellington, hoever well-intentioned, have often become self-limiting, even formulaic. Some musicians try to duplicate the sound of famous recordings; others rely upon Duke's hit songs; others nod to an Ellington line for a chorus and then go off on their own. Dan Block's way is his own. No SATIN DOLL, no transcriptions. Rather, the most familiar songs on this CD are OLD KING DOOJI and KISSING BUG. (Ask anyone who admires Ellingtonian to hum DOOJI and you'll see what I mean.) The repertoire, although not consciously esoteric, encompasses both COTTON CLUB STOMP and SECOND LINE.
Dan didn't try to find musicians who could simulate Cootie, Blanton, Greer. And while he can evoke Jimmy Hamilton, Webster, Gonsalves, Bigard, Hodges, he doesn't ever shed his own identity. Every track has its own sound — respectfully inventive. So an Ellington composition from 1940 (MORNING GLORY) is treated as if it were timeless (which it is) material for melodic improvisation, but never imprisoned by its "period" and "genre."
Duke's compositions are deeply re-imagined: KISSING BUG, which leads off, has Dan wistfully playing the line — only after he has perched atop the rattling percussion of Renato Thoms, the drums of Brian Grice, the chiming vibes of Mark Sherman, alternating with 4 /4 sections where we hear James Chirillo's guitar, Lee Hudson's bass, Mike Kanan's piano. The rhythm section work throughout — in shifting permutations — is energized without being restrictively "modern" or "traditional." Although Dan is the only horn player on this CD, I never tired of his sounds or styles.
I also noticed and applauded the natural sound of the sessions, for which I thank not only Dan but fellow saxophonist Andy Farber, who did the recording and shared mixing duties with Andrew Williams. The players whose work I knew — James Chirillo, Pat O'Leary, Lee Hudson — sound beautifully and thoroughly realized. The players who were new to me impress me thoroughly.
Each track has its own suprises — a brief but wholly musical drum solo on BUG; an unaccompanied tenor cadenza on a musing NEW YORK CITY BLUES. Dan understands that a slight shift of tempo (changing a ballad into a Fifties walk) makes a new composition although the notes seem the same.
Dan has a searching lyricism, but he also loves to rock, as I see whenever he performs. Not only does he vary his approach from performance to performance, but his horn (alto, tenor, a variety of clarinets, bass clarinet, and basset horn) without the result becoming gimmicky.
The disc is full of marvels — but three in particular stand out. One is THE BEAUTIFUL INDIANS (originally from 1947) that Dan makes into a shimmering impressionist painting through multi-tracking four reed voices (on as many instruments) — reed lines echo and intertwine, then hum and waft — all supported exquisitely by Hudson on bass and O'Leary on cello.
Another is the ambling ballad medley of ALL HEART and CHANGE MY WAYS, a track combining duets for clarinet and piano, then alto sax and piano. Mike Kanan is wondrously intuitive, his lines gliding from one beautiful voicing to the next.
But I marvel the most at the pensive A PORTRAIT OF BERT WILLIAMS reconsidered at a slightly faster tempo as a four-minute chamber piece for Dan, bass clarinet; Chirillo, guitar; O'Leary, cello; Hudson, bass. Imagine the Budapest Quartet playing Dvorak's "American" Quartet / hybridized with the Basie rhythm section, with a touch of Lucky Thompson, Oscar Pettiford, and Skeeter Best . . . that would hint at this irresistible performance. (Chirillo's acoustic playing is both funky and delicate.) This quartet returns for a sweetly lamenting ROCKS IN MY BED which reminds me of Jimmy Giuffre, Pee Wee Russell, and Danny Barker: you'll understand when you hear it.
But this disc is full of pleasures, some instantly apparent, some appearing only on repeated hearings. The music honors Ellington but no one is subsumed into an already-established idea of "Ellingtonia." And the title says a great deal: Dan and friends play approach Ellington's music by finding revelations within it.
The disc costs $20. To order yours, email its creator at BlockDan@aol.com.
Tagged Andrew Williams, Andy Farber, Barney Bigard, Basie rhythm section, bass clarinet, basset horn, Ben Webster, Bert Williams, Brian Grice, Budapest Quartet, Cootie Williams, Count Basie, Dan Block, Danny Barker, Duke Ellington, Dvorak, Emma Block, James Chirillo, jazz blog, Jazz Lives, Jimmy Blanton, Jimmy Giuffre, Jimmy Hamilton, Jo Jones, Johnny Hodges, Lee Hudson, Lucky Thompson, Mark Sherman, Michael Steinman, Mike Kanan, Mike Kawan, Oscar Pettiford, Pat O'Leary, Paul Gonsalves, Pee Wee Russell, Renato Thoms, Skeeter Best, Sonny Greer

redpajama_set_name: RedPajamaCommonCrawl


text:
Q: how to remove slash from url with htaccess how to redirect trailing slash from URL i want remove slash from end and romove slash between FILENAME
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A: RewriteRule htaccess to always remove trailing slash even directory
Try To Use The Code Below -
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redpajama_set_name: RedPajamaStackExchange


text:
INSIDE ◾BLACK◾ IOWA
Zoombombers hack meeting with Black legislators, flash image of monkey, the N-word, days before Iowa legislature reconvenes
Trolls used the image of a monkey and the N-word to disrupt a virtual meeting convened to increase public participation in the 2022 Iowa legislative session.
Black Iowa News
Editor's note: This story contains discussion of and images with racial slurs. On one image, the thumbnail has been obscured. The N-word was used in the story and headline because it is important for readers to know exactly what is happening in Iowa and being experienced by its people.
Get exclusive content. Subscribe to Black Iowa News.
Trolls interrupted the Des Moines People's Condition of the State, attended by at least three Iowa legislators, hosted by the chair of the Iowa Democratic Black Caucus. The meeting, held via Zoom, was designed to stress the importance of public participation and explain how the public can become more active in legislative processes and took place ahead of the start of the 2022 Iowa legislative session on Jan. 10.
Al Womble, chair of the Iowa Democratic Black Caucus. Womble is also state political director of the Iowa Federation of Labor, AFL-CIO. Photo courtesy of Womble.
Iowa State Rep. Phyllis Thede (D-Bettendorf) was in the middle of a presentation during the meeting describing how the public can communicate with legislators and participate in political processes when a troll interrupted with noises and flashed an image of a monkey on the screen.
Thede said: "That was absolutely awful. I'm so sorry," before continuing with her presentation.
In an interview with Black Iowa News, Thede said the racist act seemed to last forever. She said she has been called a racial epithet before but had never experienced "anything like" what occurred on Friday's call.
"To me, it's a hate crime. Whether you do it in person, or whether you do it over Zoom, or whether you send a letter in the mail, it's all a hate crime to me. And that's the way I'm looking at this because I believe that's what they were trying to get across . . . using the N-word and, you know, calling us names, they believe they achieved something, but they haven't."
Iowa State Rep. Phyllis Thede (D-Bettendorf). Photo courtesy of Thede.
Thede was able to get through the points she wanted to make, but she said people didn't get to ask as many questions as they likely would have.
Womble said he plans to turn a recording of the meeting over to the authorities. He said zoombombing is a form of violence and a public safety concern.
Iowa Democratic Chair Ross Wilburn, who was in attendance, received threats, including lynching, and was called the N-word repeatedly last year after he wrote an opinion piece for the Des Moines Register criticizing the Republican Party of Iowa and former president Donald Trump just days before a Trump rally on Oct. 9 at the Iowa State Fairgrounds.
Womble last February hosted an online meeting for the Iowa Democratic Black Caucus that was disrupted by racist trolls who spouted the "N-word and White Power" and another held by legislators was disrupted.
Friday's meeting included about 30 attendees and began at 6 p.m. The disruptions included:
A photo of a monkey and laughing
A derivative of the N-word was scribbled on Womble's screen share of the Iowa Legislature home page
Flash of a woman's image and noises
In the chat feature, someone using the name Carmen Perez wrote: "White N-word STFU" and "N-word Shut the F**k Up"
Screenshot of Zoom meeting by Black Iowa News.
A meeting participant said, "Al, do you see that?" after the monkey image flashed. Others said to block the intruder before the troll stated he didn't need to be blocked and would leave.
"It's very threatening to people who are on the call," Womble said. "These are people who are trying the best they can to disrupt the Democratic Caucus . . . They invade our platforms with obscene imagery, foul language and racial slurs and that cannot be allowed to continue."
The meeting did not require participants to pre-register, which Womble said was an oversight on his part. He said the meeting, advertised on Facebook, was open to anyone with the hopes of increasing participation. He said he doesn't know how people are able to hack into the meetings but would look for ways to improve meeting security.
"I have concern for not only the safety of my participants, but also their mental well-being, obviously, seeing things like this and hearing things like this can be very, very disturbing to people," Womble said.
On the call, Womble apologized to participants. He thanked Thede for continuing her presentation with "such grace."
"It just once again shows the maturity and the mentality of the people that we're having to deal with," he said to participants about the trolls.
In February, the Iowa Democratic Black Caucus was zoom bombed. During the meeting, U.S Rep. Joyce Beatty (D-Ohio) was speaking. Womble said information about that meeting was turned over to Capitol Police and the FBI, but he is unaware of the status of the investigation.
Screenshot from the meeting by Black Iowa News. (The image associated with the name has been obscured.)
During Friday's meeting, Thede had placed her personal phone number in the chat, which worried Womble.
Thede said she is also concerned about putting her phone number in the chat.
"Yes, I absolutely am. I absolutely am, and I'm sorry I did that," she said.
Zoom bombing, the act of interrupting virtual meetings, has gained popularity during the coronavirus pandemic as the nation relied more on virtual calls. Zoom is involved in a class-action lawsuit over its security protocols.
Just last month, trolls interrupted a school board meeting in Washington and where a troll played a recording of the N-Word and displayed a photo of George Floyd, the Minnesota man killed by police. Other virtual meetings held by state and city officials in Iowa have also been disrupted.
Womble said the trolls won't win.
"It's a shame that we have to face stuff like this. But, you know, for those people out there who don't want us to vote, and don't want us to participate in the Democratic process, they're going to try everything they possibly can to stop our community," he said. "And you know, if we hold strong, it ain't gonna stop us."
Banner: Iowa Capitol by Black Iowa News
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text:
The pear on the life of Steve Jobs opens this Saturday
The opera based on the life of former Apple CEO and co-founder of the company, Steve Jobs, is about to be released in Santa Fe (New Mexico) this Saturday. The work is called The (R) evolution of Steve Jobs and its world premiere will be on July 22 at 20:30, on the summer stage of the Santa Fe opera. Therefore, the work will be performed outdoors.
The opera had been in development since 2015. It was created by electronic music DJ Mason Bates with librettist Mark Campbell. The play tells the story of Steve Jobs and his struggle to balance life, family and work. In addition, the performance is accompanied live by an orchestra, a guitarist and natural sounds, which are complemented by electronic music and Apple's own sound devices.
Bates described one of the scenes for ABC News in a interview last week, highlighting the moment in which Steve Jobs presents the first iPhone before being defeated by the disease. At this time of Mason Bates' opera, 'The (R) Evolution of Steve Jobs', a heartbreaking sound emerges from the orchestra pit, a descending crushing progression described in the score as an 'electronic cut.'
"It's a combination of a stand-alone synthesizer with the real sound on the old Mac of hard drives when shutting down and one in the opposite direction the start ", explained Bates in an interview last week at the Opera Palace in Santa Fe, where his work will finally see the light and will be released before the public next Saturday.
"That moment is when he realizes his mortality, so he wanted to have that kind of sound accompanying him, as if off," Bates said. "Even if you can't recognize the sound, this add some authenticity since the individual, who is the subject of this opera, is the creator of some of the devices we are listening to at that time. "
The opera, which has an approximate duration of an hour and a half, begins with a prologue in the garage of the Steve Jobs family house in Los Altos, California, with the father of the protagonist, Paul Jobs, giving your child a workbench. From there, it jumps until 2007, where Jobs presents the first iPhone and then moves back in time and then back forward between 2007 and the first years of Jobs in full development of Apple. Campbell and Bates, who say that the opera is not intended to vilify or glorify the figure of Steve Jobs, have directed the work by a timeline detached from the chronological that has been imposed by emotion and memory on the figure of the genius who created Apple. The story has, in addition to the indispensable figure of Steve Jobs, with several secondary characters such as Apple co-founder, Steve Wozniak, Laurene Powell Jobs, and Chrisann Brennan, with each character highlighted through a unique series of sounds.
The (R) evolution of Steve Jobs It has been financially backed by opera companies in San Francisco and Seattle, ensuring in return a representation in the future of this avant-garde opera in California and Washington. Since his death in 2011, the life of Steve Jobs has been object of innumerable books, films and documentaries, including one directed by Danny Boyle, who wrote Aaron Sorkin. This film, which premiered in 2015 was a great success at the film box office. Since the death, the figure of the co-founder of the most important technology company in history, along with Microsoft, has been the target of multiple forms of economic exploitation. The future will tell the result of this new opera, but what is certain is that it will not be the last work based on the life of Jobs.
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text:
Q: @ElementCollection @CollectionTable in One to Many mapping I am trying relationship between in JPA using Embedded annotation, but i am not able to run it successfully,
Here my Database sql Script is as follows,
create table TBL_COLLEGE(
   id integer primary key generated always as identity (start with 1000, increment by 5),
   name varchar(50)
)

create table TBL_COURSE(
   Id  integer primary key generated always as identity (start with 10, increment by 1),
   college_Id integer references TBL_COLLEGE,
   name varchar(50)
)

here is the code below for JPA,
@Embeddable
public class Course {
...
...
..
@Id
@GeneratedValue(strategy= GenerationType.IDENTITY)
@Column(name="ID")
private Integer courseId;

@Column(name="NAME")
private String courseName;

@Column(name="COLLEGE_ID")
private Integer collegeId;
....
// getter and setter
}

Here is the College mapping,
@Entity
@Table(name="TBL_COLLEGE")
public class College implements Serializable{
   @Id
   @GeneratedValue(strategy= GenerationType.IDENTITY)
   @Column(name="ID")
   private Integer collegeId;

   ...
   ..
   @ElementCollection(targetClass=Course.class,fetch= FetchType.LAZY)
   @CollectionTable(name="TBL_COURSE",joinColumns=@JoinColumn(name="COLLEGE_ID"))
   private Set<Course> course;
   ..
   // getter and setter
}

But if i try to persist College with Courses collection set,
it gives me an exception,
ERROR: HCANN000002: An assertion failure occurred (this may indicate a bug in Hibernate)
org.hibernate.annotations.common.AssertionFailure: Declaring class is not found in the inheritance state hierarchy: com.entities.Course

....
..

Can you please tell me whether my approach is wrong,
Or my understanding for @CollectionTable is still minimal,
Were i am going wrong

A: Because both of your tables have their own ID columns, Hibernate will want them to both be @Entity types.  @Embeddables do not have their own ID.  So, first step is to change Course to be @Entity, with corresponding @TableName, etc.
This leads to the second issue, which is that the collection of Course objects shouldn't be an @ElementCollection, it should be a @OneToMany entity collection, with a @JoinColumn specifying that COLLEGE_ID will is the foreign key from TBL_COURSE.
Finally, by having a collection of Course in College, as well as a College id in Course, you are implying that you want a bidirectional association.  Among other impacts of that, you should not have the ID of the college in Course.  You should simply have the College reference.  If you don't need to navigate from Course->College, you may want to remove that for now, until you've gained a better understanding of Hibernate's object mapping.

A: Though my approach is not proper but still it worked with some minor changes in the code,
first of all i dropped the table TBL_COURSE and created a new one, as follows,
create table TBL_COURSE(
   college_Id integer references TBL_COLLEGE,
   name varchar(50)
)

here you can see i have removed the primary key, now there is only reference key and name,
Now in Course.java, i did following,
@Embeddable
public class Course {

// constuctor

@Column(name="NAME")
private String courseName;
..
// setter getter
}

Here i have removed @Id annotation and id property,i have even removed the College_Id mapping,
and the rest of the code is same as present in College.java,
And it worked,
Waiting for the opinions

A: You have to define the join about two pojo
@OneToMany
@JoinColumn(name=course table column id)
private Set<Course> course;


Brothers: John Stockton Dalgarno and Frederick Joseph Dalgarno.
P Dalgarno was listed on the Swimming Club Roll of Honour, 25 November 1916.
The youngest of the Dalgarno brothers and of a small number that served in the first three major conflicts in which Australians were involved.
He spent 131 days in South Africa during te Boer War with the Imperial Light Horse (British) after travelling at his own expense . He enlisted at Pietermaritzburg 20.2.1902 and was discharged 25.6.1902 at Johannesburg; time expired following the cessation of hostilities. His mother was shown as next of kin, again at 63 Derham St. Port Melbourne.
He enlisted August, 1914 and served WW1 as Lance Corporal, 26 Australian Army Service Corps, then listed as a 30 year-old ironmonger with his wife in Elsternwick. If his age was correctly shown, he would have been barely 18 when he travelled to South Africa to enlist in 1902.
In WW2, he enlisted from Geelong in July, 1940 and served as a Sergeant at Army HQ in Melbourne and appears to have a permanent member of the Armed Services, not being discharged until August, 1952 when he must have been around 70 years of age. Born Williamstown, 1882, died 1965 at 83 years of age in Heidelberg Repatriation Hospital, interred Springvale Crematorium.


Quilters create works of art that are also practical as bed coverings or home decoration. A quilter's handiwork can become someone else's heirloom when a sales transaction occurs. Selling handmade quilts can be done in person or through the internet. Some quilters have even found that taking custom orders is their favorite sales method. Make money with your quilting craft when you follow these steps to sell handmade quilts.
Identify upcoming quilt shows in your area from the show and events calendars provided by the American Quilter's Society and National Quilting Association (links in Resources section). Complete the seller's application for each show at which you wish to sell. Include a check for the seller's fee and mail it to the show organizer. Watch for deadlines---most shows require registration at least three months in advance.
Attach price tags to each quilt and wrap the quilts in protective plastic to transport to the quilt show. Arrive early to set up. Arrange quilts for sale on a clothing rack or tabletop so that show attendees can see the pattern and quality.
Interact with show attendees by telling them about the pattern, the process of making quilts and ask how they might use the quilt. Accept cash payments or checks with full identification.
Take digital photographs of each quilt for sale. Include shots of the full quilt, detail of the fabric patterns and a close-up of some of the quilt stitching.
Sign up as a seller on an online sales site such as eBay or Etsy.com (links in Resources section). Upload the quilt pictures onto the sale site. Add a full description including the size, quilt pattern, type of fabric and filling used and care instructions. Assign a price and list how packing, shipping and insurance fees will be charged.
Answer any email questions from prospective customers fully and in a friendly tone. Process each purchase quickly and ship the handmade quilt as soon as possible.
Print up business cards with a photo of your favorite colorful handmade quilt. Include your name, phone number and email address. Add an inviting marketing phrase like "Lovingly Handmade Quilts" or "Custom Quilts for Your Home." Give several business cards to friends and family so that they can hand them out.
Make a scrapbook or photo album of quilts you have made. Use this to show prospective customers your handiwork. Include copies of patterns that they can select from when they order the quilt.
Take a deposit when a customer places an order. Work quickly and with care to finish the quilt within the agreed timeframe. Update the customer if there are any delays. Obtain the balance of payment before turning of the quilt to the customer. Ask each satisfied customer for a note or letter to add as a testimonial to show future prospective customers.


text:
Volquez finalizes 2-year, $22M deal with Marlins
1hDavid Schoenfield
Boone tossed after rant: My guys are savages
Dodgers fuming after Phils' Neris curses them out
Catch-22: Reds scramble to fill spot after injuries
Mo wasn't afraid to chew out 'somebody who needed it. Like me': A-Rod on Mariano Rivera
1dAlex Rodriguez as told to Buster Olney
A-Rod on new Hall of Famer Edgar Martinez: 'He would have a Ph.D. in hitting'
Passan: 10 things to watch in the two weeks prior to the MLB trade deadline
2dJeff Passan
Edinson Volquez finalizes $22 million, 2-year contract with Marlins
MIAMI -- Right-hander Edinson Volquez has finalized a $22 million, two-year contract with the Miami Marlins after passing his physical.
The 33-year-old right-hander helped pitch the Kansas City Royals to the World Series title in 2015 as he went 13-9 with a 3.55 ERA. He slipped to 10-11 with 5.37 ERA with the Royals this year.
He assured everyone Friday that he is now rested and ready to go after four consecutive seasons with more than 30 starts.
"I pitched a lot of innings the year before," Volquez said in Spanish, referring to the 200 1/3 innings he threw in 2015. "By June and July (of 2016), I was tired."
Volquez joins a rotation shaken by the loss of ace Jose Fernandez, who died in a boating accident a week before the end of the regular season in September.
"It's hard to believe," Volquez said. "I was with the Royals when it happened. A lot of us were crying.
"Jose's death was a sad moment for MLB. He was a great pitcher, and he was only 24. But I don't want to be Jose. I want to be me."
An All-Star in 2008 with Cincinnati, Volquez has an 89-79 record in 12 major league seasons. He became a free agent this month when he declined his mutual option with the Royals.
Volquez said he has lived in Miami for three years, and he told his agent that becoming a member of the Marlins was his top priority in free agency.
"I've liked the Marlins team for a long time," Volquez said. "I know a lot of the guys here like Martin Prado, Dee Gordon and Marcell Ozuna. Fitting in to this clubhouse won't be a problem."
Marlins general manager Michael Hill said he was "excited" to get Volquez.
"He's a World Series champion and an All-Star," Hill said. "He will fit in perfectly with our inventory. But we are not done yet. We want to add to our pitching depth."


text:
Behavioral Health: A market ripe for growth and consolidation
Over the past six years, a number of unprecedented changes have occurred in the behavioral health market that are spurring anticipated growth and expected consolidation in the industry in the coming months. The number of covered lives is growing faster than the availability of services to treat them – creating compelling investment opportunities, as demand is significantly outstripping services supply.
The initial and primary motive for increased demand and reimbursement for behavioral health services occurred in 2008 when Congress passed the Mental Health Parity and Addiction Equity Act (MHPAEA). This act requires that insurers equalize coverage for behavioral health and medical health benefits in terms of co-pays, deductibles, lifetime caps and access to providers. Also in 2008, Congress passed the Medicare Improvements for Patients and Providers Act (MIPPA), which increased access to mental health in Federal programs. In 2013, Congress issued clarifying legislation imposing penalties and sanctions on insurers that did not comply with these requirements. In 2010, the Affordable Care Act (ACA, Obamacare) allowed adult children aged 18 through 26 to remain on their parents' insurance. It also built on MHPAEA with the requirement that most insurance plans cover mental health and substance abuse services – the largest expansion of such coverage in a generation. These major changes in reimbursement and confluence of regulatory events have resulted in marked improvements in the financing of behavioral health. 1
While financing for behavioral healthcare services has improved, the pool of qualified providers – specifically psychiatrists, particularly those certified in addiction treatment – is rapidly shrinking 2. Given this supply/demand imbalance, the market is ripe for growth. Further, the behavioral health market is fragmented and overwhelmingly dominated by small providers with no national footprint. By some estimates, only a small fraction of mental healthcare is delivered by large national providers. Private equity-based roll-ups of smaller providers therefore may be able to drive significant economies of scale, resulting in both clinical and administrative standardization. In other areas of the healthcare market, such standardization has resulted in improved health outcomes and decreased costs.
Another driver of interest in this market is the fact that psychiatric hospitals have markedly streamlined billing structures, typically billing for only 15 to 17 diagnosis-related groups (DRGs), unlike acute-care hospitals, which may bill as many as 800 DRGs. Thus, issues of clinical documentation and justification as well as inadvertent billing errors and contested billings are far less prevalent.
Given the ease of billing, supply/demand imbalance and newly mandated insurance coverage for millions of new patients, it is not surprising that it is common for behavioral health programs to have financial margins of 20% to 30%. Further, due to the chronicity of the diseases treated, these revenue streams are secure. For example, patients treated for opioid abuse frequently require chronic mental health consolation and treatment with drugs such as naltrexone, methadone or buprenorphine.
The Market Is Large
The Federal Substance Abuse and Mental Health Services Administration (SAMHSA) estimates that fully 23.9 million Americans over age 12 were addicted to or abused drugs or alcohol in the year they were surveyed. 3 Diseases such as autism spectrum disorder affect one in 68 children. 4 Clinically significant eating disorders affect 20 million women and 10 million men in the United States. 5 One in three seniors dies with Alzheimer's or another dementia. 6 The National Institute of Mental Health estimates that 9% of the U.S. population suffers from personality disorders including major clinically significant depression, schizophrenia, bipolar disorder et al.8
The advent of cognitive behavioral therapy and applied behavioral therapy has resulted in the realization that some of these disorders are amenable to clinical amelioration. The advent of tele-psychiatry and software-based clinical interventions has also resulted in a recognition that consolidation of small one-off providers can result in more efficiency and profitability. Recently, we have also seen some of the largest payers and coordinators of behavioral care, such as Magellan, beginning to adopt internet-based therapy modules.
Looking Ahead: Integration Will Drive New Growth
The behavioral health and medical care delivery systems have long been separate. However, we're starting to see more of a push to integrate the two. This is true particularly where state and federal programs are encouraging proactive integration to reduce emergency room admissions and readmissions: Approximately 75% of high-users of hospital inpatient services have behavioral health diagnoses. 7 Therefore, in 2015, BDO expects to see continued changes in efforts to increase behavioral health service capacity and better integrate it with clinical care through more formal affiliations, partnerships and merger activity.
We envision this integration happening both voluntarily and via mandates similar to the Medicaid Redesign/Delivery System Reform Incentive Payments (DSRIP) program in New York state and California. Such integration of physical and mental health providers will result in the screening and identification of even more patients who will have insurance coverage for behavioral health issues resulting in an increased demand over and above what has been seen thus far.
The clinical care of behavioral health issues such as substance abuse, attention deficit disorder, autism and eating disorders has arrived at a crucial nexus. Significant new funding is available to providers skilled in treating these disorders. Simultaneously, there are fewer providers with the appropriate skill sets required to treat these patients. While potential threats to Obamacare are currently being lodged by the new congressional majority, BDO believes that while the ACA may be modified, it is unlikely to be repealed. Over the next five years, we envision more and more consolidations, mergers and acquisitions in this field as investors recognize the unique confluence of investment opportunities inherent in a market dominated by small niche behavioral health programs. As these programs join together, they will be able to create value for patients, communities and investors. The efficiencies created should result in improved care delivered by highly profitable, clinically excellent programs.
1 McGuireWoods LLP, and HCP & Co. Bullish Behavioral Health Market Drives Investment. New York: Law360, 2014. Web. 27 Jan. 2015.
2 Thomas, Kathleen et al. 'County-Level Estimates Of Mental Health Professional Shortage In The United States: Psychiatric Services: Vol 60, No 10'. Psychiatryonline.org. N.p., 2009. Web. 27 Jan. 2015.
3 SAMHSA, Center for Behavioral Health Statistics and Quality, National Survey on Drug Use and Health, 2013
4 CDC.gov. "Prevalence of Autism Spectrum Disorder among Children Aged 8 Years – Autism and Developmental Disabilities Monitoring Network, 11 Sites, United States, 2010" Web. March 27, 2014.
5 Wade, T. D., Keski-Rahkonen A., & Hudson J. (2011). Epidemiology of eating disorders. In M. Tsuang and M. Tohen (Eds.), Textbook in Psychiatric Epidemiology (3rd ed.) (pp. 343-360). New York: Wiley
6 Asha.org. 'Dementia: Incidence And Prevalence'. Web. 27 Jan. 2015.
7 Chakravarty, Sujoy et al. Role Of Behavioral Health Conditions In Avoidable Hospital Use And Cost. New Brunswick: Rutgers Center for State Health Policy, 2014. Web. 27 Jan. 2015.
8 Lenzenweger MF, Lane MC, Loranger AW, Kessler RC. DSM-IV personality disorders in the National Comorbidity Survey Replication . Biol Psychiatry. 2007 Sep 15;62(6):553-64.
Dr. Bill Bithoney is a leading physician executive, with experience running an integrated healthcare delivery system, including an award-winning ACO, as an Interim President & Chief Executive Officer (CEO), Chief Operating Officer (COO) & Chief Medical Officer (CMO) of Sisters of Providence Health System (SPHS). In these roles, he oversaw operations of five hospitals – which included Providence Behavioral Health Hospital. As COO and CEO, he managed their Substance Abuse, Methadone Maintenance and Behavioral Health Programs.
About The BDO Center for Healthcare Excellence and Innovation
The BDO Center for Healthcare Excellence & Innovation unites recognized industry thought leaders to provide sustainable solutions across the full spectrum of healthcare challenges facing key stakeholders. Leveraging deep healthcare experience in financial, clinical, data analytics and regulatory disciplines, we deliver research-based insights, innovative approaches and value-driven services to help guide efficient healthcare transformation to improve the quality and lower the cost of care. BDO understands the unique accounting, financial, clinical, data and regulatory requirements that demand experienced attention to help organizations achieve growth and sustainability in today's evolving marketplace.
Article March 31, 2015
6 Steps to Check Up On: Organizational Transformation & Margin Improvement in Healthcare
December 20, 2022
Today's market environment has created some difficult challenges for healthcare organizations with 69% of health system strategic planners reporting operating margins below pre-pandemic performance in 2022.
2022 BDO Patient Experience Survey
To help providers better understand this new environment, we conducted the 2022 BDO Patient Experience Survey, which polled 3,000 U.S. adults on their feelings towards their providers, insurance and overall healthcare experience.


text:
\section{introduction}
\par
Optical lattice is an artificial lattice produced by standing wave of
laser light\cite{Pitaevskii}. In a cold atom gas loaded on an optical
lattice, atoms feel a periodic potential due to the Stark effect. When
the lattice potential is strong, this system can be well described by
the Hubbard model, where atoms are hopping between nearest-neighbor
sites, interacting with each other when they meet at the same lattice
site. Since the Hubbard model is a fundamental model in condensed matter
physics, it is expected that various topics discussed in this field may
be solved by using the optical lattice system. Indeed, the
superfluid-Mott insulator transition has been observed in a $^{87}$Rb
lattice Bose gas\cite{Greiner,Esslinger}. More recently, the superfluid
state has been also realized in a $^6$Li lattice Fermi
gas\cite{chin06,Miller}.
\par
Besides the optical lattice, a tunable interaction associated with a
Feshbach resonance is also an advantage of cold atom
gases\cite{Timmermans,Holland}. Using this unique property, several
experimental groups\cite{Jin,Grimm,Ketterle,Thomas} have succeeded in
realizing Fermi superfluids and the BCS-BEC (Bose-Einstein condensation)
crossover\cite{Leggett,Nozieres,Tokumitu,Melo,Haussmann94,Haussmann,Ohashi,Levin}
in the absence of optical lattice. The BCS-BEC crossover is a very
interesting phenomenon, because one can study the weak-coupling
BCS-state and the BEC of tightly bound molecules in a unified manner by
varying the strength of a pairing interaction. Since this tunable
pairing interaction also works in an optical lattice, it is interesting
to examine how the BCS-BEC crossover phenomenon is observed in the
optical lattice system. We briefly note that, in the Hubbard model,
interaction effects are parametrized by the scaled interaction $U/t$
(where $U$ and $t$ represent an on-site pairing interaction and
nearest-neighbor hopping, respectively). Thus, in addition to the direct
tuning of the pairing interaction by a Feshbach resonance, continuous
change from the weak- to strong-coupling regime can be also realized by
adjusting the hopping parameter $t$ by tuning the intensity of laser
light producing the optical lattice.
\par
The BCS-BEC crossover in the attractive Hubbard model has been discussed
in superconductivity literature\cite{Micnus}, in connection to
strongly-correlated electron systems. Nozi\`eres and
Schmitt-Rink\cite{Nozieres} pointed out the mass enhancement of tightly
bound molecules in the strong-coupling BEC regime, because of virtual
dissociation of a bound molecule during hopping between lattice
sites. This mass enhancement is expected to decrease the superfluid
phase transition temperature $T_{\rm c}$ in the BEC regime, which has
been theoretically confirmed by the self-consistent $t$-matrix
theory\cite{keller99}, dynamical mean-field theory\cite{keller01}, and
quantum Monte-Carlo simulation\cite{sewer02}. Competition between
pairing fluctuations and charge density wave (CDW)
fluctuations\cite{note} near the half-filling (which comes from the
nesting property of the square-shape Fermi surface at the half-filling)
has been also studied\cite{taraph95}. In two-dimension,
Refs. \cite{Scalettar,deisz02} pointed out that this competition leads
to vanishing $T_{\rm c}$ at the half-filling. For more details, we refer
to Ref. \cite{Micnus}.
\par
In this paper, we investigate the superfluid phase transition in a gas
of Fermi atoms loaded on a three-dimensional cubic optical
lattice. Treating this system as the Hubbard model, we calculate $T_{\rm
c}$ in the BCS-BEC crossover region, including pairing fluctuations, as
well as CDW and spin density wave (SDW) fluctuations in a consistent
manner within the self-consistent $t$-matrix approximation
(SCTA)\cite{Haussmann94,Haussmann,engel02} and fluctuation exchange
approximation (FLEX)\cite{deisz02}, respectively. Our theory satisfies
the required particle-hole symmetry over the entire BCS-BEC crossover
region. While a finite $T_{\rm c}$ is obtained at the half-filling in
contrast to the two-dimensional case\cite{Scalettar}, the superfluid
phase transition is shown to be strongly influenced by CDW fluctuations
near the half-filling. The resulting $T_{\rm c}$ takes the maximum
value, not at the half-filling, but around the quarter filling. Since
strong CDW fluctuations are characteristic of the lattice system we
consider in this paper, the observation of the filling dependence of
$T_{\rm c}$ would be an interesting problem.

\par
This paper is organized as follows. In Sec. II, we explain our
formulation. The self-consistent $t$-matrix approximation (SCTA) for
pairing fluctuations and the fluctuation exchange approximation (FLEX)
for CDW and SDW fluctuations are explained. In Sec. III, we present our
numerical results for the superfluid phase transition temperature, only
taking into account pairing fluctuations. We examine effects of CDW and
SDW fluctuations on the superfluid phase transition in
Sec. IV. Throughout this paper, we set $\hbar=k_B=1$.

\section{Formulation}
\par
We consider a two-component Fermi gas in a three-dimensional cubic
optical lattice. In superfluid Fermi gases, all the current experiments
are using a broad Feshbach resonance\cite{Jin,Ketterle,Grimm,Thomas}. In
this case, details of the Feshbach resonance is known to be not
important as far as we consider the interesting BCS-BEC crossover
region, so that we can safely consider this system using the ordinary
BCS model. In addition, as mentioned in the introduction, a Fermi gas in
an optical lattice can be well described by the Hubbard model when the
lattice potential is strong. Under these conditions, we consider the
attractive Hubbard model described by the Hamiltonian
\begin{eqnarray}
H=-t\sum_{(i,j),\sigma}(c^{\dagger}_{i,\sigma} c_{j,\sigma}
 + \mathrm{h.c.})-U\sum_{i}n_{i\uparrow}n_{i\downarrow}
 - \mu\sum_{i,\sigma} n_{i,\sigma}.
 \label{eq.1}
\end{eqnarray}
Here, $c_{j,\sigma}$ is the annihilation operator of a Fermi atom at the
$j$-th lattice site, where the pseudo-spin $\sigma=\uparrow,\downarrow$
describes two atomic hyperfine states. $t$ is the hopping matrix element
between nearest-neighbor sites, and the summation $(i,j)$ in the first
term is taken over nearest-neighbor
pairs. $n_{i\sigma}=c^\dagger_{i\sigma}c_{i\sigma}$ is the number
operator. The on-site pairing interaction $-U~(<0)$ is implicitly
assumed to be tunable by using a Feshbach resonance. $\mu$ is the Fermi
chemical potential. In Eq. (\ref{eq.1}), we have neglected effects of a
harmonic trap, for simplicity.
\par
\begin{figure}
\includegraphics[scale=1.3]{fig1}
\caption{
Self-energy corrections describing (a) pairing fluctuations, (b) CDW fluctuations and SDW fluctuations of the $z$-component, and (c) SDW fluctuations of the $x$- and $y$-component. The solid line and dashed line describe the single-particle Green's function $G$ and the attractive interaction $-U$, respectively.
\label{fig1}
}
\end{figure}
\begin{figure}
\includegraphics[scale=0.6]{fig2}
\caption{
Vertex functions of (a) particle-particle channel $\Gamma_{\rm pp}$ and (b), (c) particle-hole channel $\Gamma_{\rm ph}^{\rm s,d}$. In our calculation, the lowest order term in terms of $U$ is included in $\Gamma_{\rm pp}$.
 \label{fig2}
}
\end{figure}
\par
We calculate the superfluid phase transition temperature $T_{\rm c}$,
extending SCTA developed by Haussmann\cite{Haussmann94,Haussmann} so as to
include CDW and SDW fluctuations within FLEX. Effects of these
fluctuations are described by the self-energy $\Sigma({\bm
k},i\omega_m)$ in the single-particle Green's function $G({\bm
k},i\omega_m)$,
\begin{equation}
G(\bm{k},i\omega_m)=
{1 \over
i\omega_m-\varepsilon_{\bf k}+\mu-\Sigma({\bf k},i\omega_m)},
\label{eq2}
\end{equation}
where $\varepsilon_{\bf k}\equiv-2t[\cos k_x+\cos k_y+\cos k_z]-\mu$ is
the kinetic energy of a Fermi atom measured from the chemical potential
$\mu$ (where the lattice constant is taken to be unity). $\omega_m$ is
the fermion Matsubara frequency.
\par
Figure \ref{fig1}(a) shows the self-energy correction coming from
pairing fluctuations ($\equiv \Sigma_{\rm pp}$). Summing up this type of
diagrams within SCTA, we obtain
\begin{equation}
\Sigma_{\rm pp}({\bm k},i\omega_m)=
{1 \over \beta}\sum_{{\bm q},i\nu_n}
\Gamma_{\rm pp}({\bm q},i\nu_n)G({\bm q}-{\bm k},i\nu_n-i\omega_m),
\label{eq3}
\end{equation}
where $\nu_n$ is the boson Matsubara frequency.
Hereafter, the factor $1/N$ of lattice sites number in front of momentum
summation is abbreviated for simple presentation.
$\Gamma_{\rm pp}$ is the particle-particle scattering vertex diagrammatically described by Fig.\ref{fig2}(a). The result is
\begin{equation}
\Gamma_{\rm pp}({\bm q},i\nu_n)=
-{U \over 1-U\Pi_{\rm pp}({\bm q},i\nu_n)},
\label{eq4}
\end{equation}
where,
\begin{equation}
\Pi_{\rm pp}({\bm q},i\nu_n)=
{1 \over \beta}\sum_{{\bf k},i\omega_m}
G({\bm k},i\omega_m)G({\bf q}-{\bm k},i\nu_n-i\omega_m)
\label{eq5}
\end{equation}
is a correlation function describing fluctuations in the Cooper channel.
\par
In Fig.\ref{fig1}, panels (b) and (c) describe fluctuations in the
particle-hole channel within FLEX. Panel (b) involves both CDW
fluctuations and longitudinal SDW fluctuations. Panel (c) involves
transverse SDW fluctuations. Summing up these diagrams, we obtain the
self-energy corrections associated with CDW fluctuations $(\equiv
\Sigma_{\rm ph}^{\rm d})$ and SDW fluctuations ($\equiv \Sigma_{\rm
ph}^{\rm s})$ as
\begin{eqnarray}
\Sigma_{\rm ph}^{\rm d,s}({\bm k},i\omega_m)
&=&
-{U \over \beta}\sum_{{\bf q},i\nu_n}
\Pi_{\rm ph}({\bm q},i\nu_n)\Gamma_{\rm ph}^{\rm d,s}({\bm
q},i\nu_n)G({\bm k}-{\bm q},i\omega_m-i\nu_n)\nonumber\\
&\equiv&
{1 \over \beta}\sum_{{\bf q},i\nu_n}
V_{\rm ph}^{\rm d,s}({\bm q},i\nu_n)G({\bm k}-{\bm q},i\omega_m-i\nu_n),
\label{eq6}
\end{eqnarray}
where $V_{\rm ph}^{\rm d,s}$ is introduced for saving the computational time by
performing the fast Fourier transformation (FFT), which is explained in Sec. III.
Here, the vertex functions $\Gamma_{\rm ph}^{\rm d}$ and $\Gamma_{\rm
ph}^{\rm s}$ are obtained from the sum of the diagrams shown in
Figs.\ref{fig2}(a) and \ref{fig2}(b), and their expressions are given by
\begin{eqnarray}
\Gamma_{\rm ph}^{\rm d}(\bm{q},i\nu_n)=
-{1 \over 2}
{
U^2\Pi_{\rm ph}({\bm q},i\nu_n)
\over
1-U\Pi_{\rm ph}({\bm q},i\nu_n)
}.
\label{eq7}
\end{eqnarray}
\begin{eqnarray}
\Gamma_{\rm ph }^{\rm s }({\bm q},i\nu_n)=
{3 \over 2}
{U^2\Pi_{\rm ph}({\bm q},i\nu_n)
\over
1+U\Pi_{\rm ph}({\bm q},i\nu_n)
}.
\label{eq8}
\end{eqnarray}
In Eqs. (\ref{eq7}) and (\ref{eq8}), the correlation function $\Pi_{\rm ph}({\bm k},i\nu_n)$ describes fluctuations in the particle-hole channel, having the form
\begin{equation}
\Pi_{\rm ph}({\bm q},i\nu_n)=-
{1 \over \beta}\sum_{{\bm k},i\omega_m}
G({\bm k},i\omega_m)G({\bf k}-{\bm q},i\omega_m-i\nu_n).
\label{eq9}
\end{equation}
The superfluid phase transition temperature $T_{\rm c}$ is determined from the Thouless criterion\cite{Haussmann94,Haussmann}, stating that the superfluid phase transition occurs when the particle-particle scattering vertex $\Gamma_{\rm pp}({\bm q},i\nu_n)$ has a pole at ${\bm q}=\nu_n=0$. Using this, we obtain the equation for $T_{\rm c}$ as
\begin{equation}
1=U\Pi_{\rm pp}({\bm q}=0,i\nu_n=0).
\label{eq10}
\end{equation}
We note that Eq. (\ref{eq10}) is affected by CDW and SDW fluctuations through the self-energy $\Sigma=\Sigma_{\rm pp}+\Sigma_{\rm ph}^{\rm d}+\Sigma_{\rm ph}^{\rm s}$ in the Green's function.
\par
In the weak-coupling BCS regime, we may set $\mu=\varepsilon_{\rm F}$ (where $\varepsilon_{\rm F}$ is the Fermi energy) in Eq. (\ref{eq10}). However, the chemical potential is known to deviate from $\varepsilon_{\rm F}$, as one approaches the strong-coupling BEC regime\cite{Leggett,Nozieres}. This strong-coupling effect is taken into account by considering the equation for the filling number $n$ (which gives the number of atoms per lattice site), given by
\begin{equation}
n={2 \over \beta}\sum_{{\bm k},i\omega_m}e^{i\omega_m\delta}G({\bm k},i\omega_m),
\label{eq11}
\end{equation}
where $\delta$ is an infinitesimal positive number. We solve the coupled equations (\ref{eq10}) and (\ref{eq11}) to determine $T_{\rm c}$ and $\mu$ self-consistently for a given $U$ and $n$.
\par
At the half-filling $n=1$, the superfluid state and CDW are degenerate in the sense that they have the same phase transition temperature\cite{Micnus,taraph95}. The CDW phase transition is characterized by the divergence of the charge susceptibility $\chi_{\rm CDW}({\bm Q})$ with the momentum ${\bm Q}=(\pi,\pi,\pi)$. In the random phase approximation, $\chi_{\rm CDW}$ is given by
\begin{eqnarray}
\chi_{\rm CDW}({\bm Q}=(\pi,\pi,\pi))=
\frac{1}{2}
\frac{\Pi_{\rm ph}({\bm Q},0)}{1-U\Pi_{\rm ph}({\bm Q},0)},
\label{eq12}
\end{eqnarray}
where the correlation function $\Pi_{\rm ph}({\bm Q},i\nu_n)$ is given by Eq. (\ref{eq9}). Comparing Eq. (\ref{eq12}) with Eq. (\ref{eq7}), we find that the CDW vertex function $\Gamma_{\rm ph}^{\rm d}({\bm Q},i\nu_n=0)$ also diverges at $T_{\rm c}$. This CDW instability at the superfluid phase transition temperature $T_{\rm c}$ is absent when $n\ne 1$ due to the absence of the perfect nesting of the Fermi surface. However, since the denominator $1-U\Pi_{\rm ph}({\bm Q},i\nu_n=0)$ in Eq. (\ref{eq12}) is still small at $T_{\rm c}$ near the half-filling, strong CDW fluctuations are expected when $n\sim 1$.
\par
In contrast, the SDW vertex function $\Gamma_{\rm ph}^{\rm s}$ in Eq. (\ref{eq8}) does not diverge at $T_{\rm c}$ even when $n=1$. Namely, spin fluctuations are weak in the attractive Hubbard model.
\par
\section{Effects of pairing fluctuations on $T_{\rm c}$ and $\mu$ in the BCS-BEC crossover region}
In the following two sections, we show our numerical results obtained by solving the coupled equations (\ref{eq10}) and (\ref{eq11}). In this section, we first consider $T_{\rm c}$ in the BCS-BEC crossover, including pairing fluctuations only. Although one cannot actually ignore strong CDW fluctuations near the half-filling, examining this simple case is still useful in considering importance of CDW and SDW fluctuations. We separately discuss effects of CDW and SDW fluctuations in Sec. IV.
\par
Before showing our results, we summarize the outline of computation. In solving the coupled equations (\ref{eq10}) and (\ref{eq11}), we use the fact that the self-energy $\Sigma=\Sigma_{\rm pp}+\Sigma_{\rm ph}^{\rm d}+\Sigma_{\rm ph}^{\rm s}$ in Eqs.(\ref{eq3}) and (\ref{eq6}), the correlation functions $\Pi_{\rm pp}$ and $\Pi_{\rm ph}$ in Eqs. (\ref{eq5}) and (\ref{eq9}), and the number equation in Eq. (\ref{eq11}) have simple expressions in real space, as
\begin{eqnarray}
\Sigma({\bm r},\tau)
&=&
\Sigma_{\rm pp}({\bm r},\tau)+
\Sigma_{\rm ph}^{\rm d}({\bm r},\tau)+
\Sigma_{\rm ph}^{\rm s}({\bm r},\tau)
\nonumber
\\
&=&
\Gamma_{\rm pp}({\bm r},\tau)G(-{\bm r},-\tau)+
\Bigl[
 V_{\rm ph}^{\rm d}({\bm r},\tau)+
 V_{\rm ph}^{\rm s}({\bm r},\tau)
\Bigr]G({\bm r},\tau),
\label{eq13}
\end{eqnarray}
\begin{eqnarray}
\Pi_{\rm pp}({\bm r},\tau)=G({\bm r},\tau)G({\bm r},\tau),
\label{eq14}
\end{eqnarray}
\begin{eqnarray}
\Pi_{\rm ph}({\bm r},\tau)=-G({\bm r},\tau)G(-{\bm r},-\tau),
\label{eq15}
\end{eqnarray}
\begin{equation}
n=2G(\bm{r}=0,\tau=-\delta).
\label{eq16}
\end{equation}
Here, ${\bm r}$ is the spatial position of a lattice site and $\tau$ is the imaginary time. The Fourier transformation is defined by
\begin{eqnarray}
\left\{
\begin{array}{ll}
\displaystyle
G({\bm r},\tau)={1 \over \beta}\sum_{{\bf k},i\omega_m}G({\bm k},i\omega_m)
e^{i({\bm k}\cdot{\bm r}-\omega_m\tau)},\\
\displaystyle
G({\bm k},i\omega_m)=\sum_{\bf r}\int_0^\beta d\tau G({\bm k},\tau)
e^{-i({\bm k}\cdot{\bm r}-\omega_m\tau)}.\\
\end{array}
\right.
\label{eq17}
\end{eqnarray}
To use Eqs. (\ref{eq13})-(\ref{eq16}), we employ the FFT method\cite{note2}. We discretize the momentum
region $0\le k_x,k_y,k_z\le\pi$ into $16\times16\times16$ cells. For the
frequency summations, we introduce a finite cutoff frequency
$\omega_{\rm max}=\pi T(2n_{\rm max}+1)$ for fermions and $\nu_{\rm
max}=2\pi T n_{\rm max}$ for boson, with $n_{\rm max}=512$. The values
of these cutoffs are chosen so as to be much larger than the band width $2zt$
(where $z=6$ is the coordination number of the simple cubic lattice), as
well as the magnitude of the pairing interaction $U$. To avoid effects
of these cutoff frequencies, we use the method discussed in
\cite{deisz02}. We explain the outline of this method in the Appendix.
\par

\begin{figure}
\includegraphics[scale=0.7]{fig3}
\caption{Superfluid phase transition temperature $T_{\rm c}$ as a function of pairing interaction $U$ and filling number $n$. In this figure, and in Fig.\ref{fig4}, we only include pairing fluctuations described by $\Sigma_{\rm pp}$. Since $T_{\rm c}$ at the filling $2-n$ is the same as $T_{\rm c}$ at $n$ due to the particle-hole symmetry, we only show the result less than half-filling ($n\le 1$).
\label{fig3}
}
\end{figure}

\begin{figure}
\includegraphics[scale=0.7]{fig4}
\caption{Chemical potential $\mu$ as a function of $U$ at $T_{\rm c}$. $\mu=-U/2$ is the exact solution at the half-filling $n=1$. At $U=0$, apart from weak temperature effect, $\mu$ is almost equal to the Fermi energy $\varepsilon_{\rm F}$ for a given filling number $n$.
\label{fig4}
}
\end{figure}

\par
Figure \ref{fig3} shows the calculated $T_{\rm c}$ in the BCS-BEC crossover. In this calculation, we only include the self-energy $\Sigma_{\rm pp}$ associated with pairing fluctuations. Since the Hubbard model  has the particle-hole symmetry, the filling dependence of $T_{\rm c}$ is symmetric with respect to $n=1$ (although we do not show it explicitly). Namely, for a given $U$, Fig.\ref{fig3} shows that the maximum $T_{\rm c}$ is obtained at the half-filling $n=1$, while $T_{\rm c}$ vanishes at $n=2$ as in the case of $n=0$.
\par
In the weak-coupling BCS regime ($U/6t\ \raise.3ex\hbox{$<$}\kern-0.8em\lower.7ex\hbox{$\sim$}\  1$), $T_{\rm c}$ is an increasing function of $U$. This behavior agrees with the well-known mean-field BCS result,
\begin{equation}
T_{\rm c}\propto t e^{-{1 \over N(0)U}},
\label{eq18}
\end{equation}
where $N(0)$ is the density of states at the Fermi level. In this regime, since $T_{\rm c}$ is comparable to the binding energy $E_{\rm bind}$ of a Cooper pair at $T=0$, the increase of $T_{\rm c}$ reflects the enhancement of $E_{\rm bind}$ as one approaches the strong-coupling regime.
\par
For a given filling number $n$, the maximum $T_{\rm c}$ ($\equiv T_{\rm c}^{\rm max}$) is obtained around the intermediate coupling region $U/6t\sim 1$. At the half-filling ($n=1$), we obtain $T_{\rm c}^{\rm max}=0.042$ at $U/6t=0.9$. $T_{\rm c}$ then decreases as one further increases the magnitude of $U$. The decrease of $T_{\rm c}$ in the BEC regime is characteristic of the BCS-BEC crossover in the Hubbard model\cite{Micnus}. In a uniform Fermi gas with no lattice potential, $T_{\rm c}$ approaches the constant value $T_{\rm c}=0.218\varepsilon_{\rm F}$ in the BEC limit\cite{Melo,Haussmann94,Ohashi}.
\par
We note that the decrease of $T_{\rm c}$ in the BEC regime does not mean the small binding energy of a bound molecule in this regime. As shown in Fig.\ref{fig4}, while the chemical potential $\mu$ is almost equal to the Fermi energy $\varepsilon_{\rm F}$ at $U=0$ (apart from weak temperature effect), it becomes smaller than the bottom of the band ($=-6t$) in the strong coupling regime. This means the existence of a {\it finite energy gap} $E_{\rm g}=|\mu|-6t$ in the Fermi single-particle excitations in the BEC regime. Since $E_{\rm g}$ is directly related to the dissociation energy of a bound molecule, we find that the binding energy $E_{\rm b}$ continues to increase even in the BEC regime (although $T_{\rm c}$ decreases as shown in Fig.\ref{fig3}).
\par
To understand physics behind the decreasing $T_{\rm c}$ in the BEC regime, it is helpful to derive an effective model valid for this regime. To do this, we note that in the BEC regime, tightly bound molecules have been already formed above $T_{\rm c}$. In this case, as pointed out in Ref. \cite{Nozieres}, molecular motion is accompanied by virtual dissociation, because each atoms in a molecule has to move one by one in the Hubbard model. In addition, this virtual dissociation also leads to a repulsive interaction between molecules\cite{Nozieres}. Including these effects within the second order perturbation in terms of the hopping $t$, we obtain the effective Hamiltonian\cite{robasz81},
\begin{eqnarray}
H_{\rm eff}=-{2t^2 \over U}\sum_{(i,j)}[b^\dagger_i b_j+{\rm h.c.}]
+{4t^2 \over U}\sum_{(i,j)}n^{\rm B}_i n^{\rm B}_j
-\mu_{\rm B}\sum_i n^{\rm B}_i,
\label{eq19}
\end{eqnarray}
where $b^\dagger_i=c^\dagger_{i\uparrow}c^\dagger_{i\downarrow}$
describes a molecule at the $i$-th lattice site, and $n^{\rm
B}_i=(n_{i\uparrow}+n_{i\downarrow})/2$ gives the number of molecules
under the assumption that all the atoms form small on-site bound
pairs. $\mu_{\rm B}=2\mu+U+2zt^2/U$ is the molecular chemical potential to control the molecular density. In Eq. (\ref{eq19}), double occupancy of molecules is forbidden due to the Pauli's exclusion principle of Fermi atoms in them. Noting this and commutation relations, $[b_i^\dagger,b_i]=2(n_i^{\rm B}-1/2)$, $[n_i^{\rm B}-1/2,b_i^{\dagger}]=b_i^{\dagger}$, and $[n_i^{\rm B}-1/2,b_i]=-b_i$, we can map Eq. (\ref{eq15}) onto the $S=1/2$ Heisenberg model, by replacing $(b_i^\dagger,b_i,n_i^{\rm B}-1/2)$ with $((-1)^iS_i^+,(-1)^iS_i^-,S_i^z)$,
\begin{equation}
H_{\rm eff}
=J\sum_{(i,j)}{\bf S}_i\cdot{\bf S}_j-h_{\rm B}\sum_iS_i^z.
\label{eq20}
\end{equation}
Here, $J=4t^2/U$ is an exchange interaction and $h_{\rm B}=\mu_{\rm B}-2zt^2/U$ works as an external magnetic field. Since $S_i^z=-1/2$ and $S_i^z=+1/2$ state in Eq. (\ref{eq16}), respectively, correspond to a vacant and occupied site in the effective model in Eq. (\ref{eq19}), the half-filling case is described by setting $h_{\rm B}=0$ in Eq. (\ref{eq20}). Equation (\ref{eq20}) clearly shows that the `N\'{e}el temperature $T_{\rm N}$' (which corresponds to $T_{\rm c}$ in the original Hubbard model) is lower for larger $U$, consistent with the decreasing $T_{\rm c}$ in the strong-coupling BEC regime shown in Fig.\ref{fig3}.
\par
The N\'{e}el temperature of the Heisenberg model has been studied by various methods. It has been shown that the mean-field result $T_{\rm N}=6t^2/U$ is suppressed by spin fluctuations to be $T_{\rm N}=3.59t^2/U$ (high temperature expansion)\cite{rush63} and $T_{\rm N}=3.78t^2/U$ (quantum Monte Carlo method)\cite{sand98}. In the present calculation, we obtain $T_{\rm c}\simeq 1.5t^2/U < (3.59\sim3.78)t^2/U$ in the BEC regime, showing that the present calculation based on SCTA underestimates $T_{\rm c}$ in the BEC regime.
\par
One reason for this discrepancy is the approximate treatment of the interaction between molecules. To see this, we consider the BCS-BEC crossover problem within the Gaussian fluctuation theory developed by Nozi\`eres and Schmitt-Rink\cite{Nozieres}. (We refer this theory as the NSR theory in the following.) In the NSR theory, one also solves the coupled equations (\ref{eq10}) and (\ref{eq11}), where the single-particle Green's function $G$ and the correlation function $\Pi_{\rm pp}$ are now replaced by
\begin{eqnarray}
G({\bm p},i\omega_m)=G_0(\bm{k},i\omega_m)
+G_0(\bm{k},i\omega_m) \Sigma_{\rm pp}(\bm{k},i\omega_m)
 G_0(\bm{k},i\omega_m),
\label{eq21}
\end{eqnarray}
\begin{eqnarray}
\Pi_{\rm pp}({\bm q},i\nu_n)={1 \over \beta}
\sum_{\bm{k},i\omega_m}
G_0(\bm{k},i\omega_m)G_0(\bm{q}-\bm{k},i\nu_n-i\omega_m),
\label{eq22}
\end{eqnarray}
where $G_0({\bf k},i\omega_m)^{-1}=i\omega_m-\varepsilon_{\bf k}+\mu$ is the Green's function in a free Fermi gas. The self-energy part in Eq. (\ref{eq21}) is given by
\begin{eqnarray}
\Sigma_{\rm pp}(\bm{k},i\omega_m)
={1 \over \beta}\sum_{\bm{q},i\nu_n}\Gamma_{\rm pp}(\bm{q},i\nu_n)
G_0(\bm{q}-\bm{k},i\nu_n-i\omega_m).
\label{eq23}
\end{eqnarray}
The particle-particle scattering vertex $\Gamma_{\rm pp}$ is given by Eq. (\ref{eq4}), where $\Pi_{\rm pp}$ is replaced by Eq.(\ref{eq22}).
\par

\begin{figure}
\includegraphics[scale=0.7]{fig5}
\caption{Calculated $T_{\rm c}$ within the NSR theory. `BCS limit' is the mean-filed BCS result with $\mu=\varepsilon_{\rm F}$. `BEC limit' shows $T_{\rm c}$ of an ideal molecular Bose gas.
\label{fig5}
}
\end{figure}
\par
Figure \ref{fig5} shows the calculated $T_{\rm c}$ based on the NSR
theory. Comparing this result with Fig.\ref{fig3}, we find that the NSR
theory gives higher $T_{\rm c}$. Since the NSR theory is a low density
approximation\cite{Nozieres} (Note that only the free propagator $G_0$ is used and the self-energy correction is only taken into account to
the first order in the number equation (\ref{eq10}).), the difference
between the two is more remarkable in higher filling cases.
\par
In the BEC limit of the NSR theory, Eq. (\ref{eq10}) gives $\mu=-U/2$, and the number equation (\ref{eq11}) reduces to the condition for BEC in an ideal Bose gas,
\begin{equation}
{n \over 2}=\sum_{\bf k}
{1 \over e^{\beta(E_{\bf q}^{\rm B}-{\bar \mu}_{\rm B})}-1},
\label{eq24}
\end{equation}
where $E_{\bf q}^{\rm B}=-2(2t^2/U)[\cos q_x+\cos q_y+\cos q_z]$ and ${\bar \mu}_{\rm B}=-6(2t^2/U)$. Indeed, Fig.\ref{fig5} shows that $T_{\rm c}$ obtained from Eq. (\ref{eq24}) well describes the NSR result in the strong-coupling regime. Noting that the kinetic energy $E_{\bf q}^{\rm B}$ can be also obtained from the first term in Eq. (\ref{eq19}) when one regards $b_i$ as a boson operator, we find that the NSR theory ignores the repulsive interaction between molecules given by the second term in Eq. (\ref{eq19}).
\par
In a uniform Fermi gas with no lattice potential, Haussmann pointed out that, in the BEC regime, SCTA includes the interaction between molecules within the Born approximation\cite{Haussmann94}. This molecular interaction can be written as $U_{\rm B}=4\pi a_{\rm B}/M_{\rm B}$, where $M_{\rm B}$ is a molecular mass. The $s$-wave molecular scattering length $a_{\rm B}$ is related to the $s$-wave atomic scattering length $a_s$ as $a_B=2a_s$. Even in the presence of the lattice, the molecular interaction is expected to be included within the same approximation level. Thus, we find that the lower $T_{\rm c}$ within SCTA than the NSR result originates from the molecular interaction. Namely, the molecular interaction lowers $T_{\rm c}$ in the BEC regime in the lattice system.
\par
Recent work\cite{Strinati,Petrov,Gio,Ohashi3} on a uniform Fermi gas has clarified that, when one carefully treats higher order molecular scattering processes and a finite value of molecular binding energy, $a_{\rm B}$ reduces to $a_{\rm B}=0.6a_s<2a_s$. This clearly indicates {\it overestimate} of the magnitude of molecular interaction in SCTA. When we apply this discussion to the present lattice system, one reason for the underestimate of $T_{\rm c}$ $( =1.5t^2/U < (3.59\sim3.78)t^2/U)$ is expected to be the overestimate of the molecular interaction. When one could correct this point, $T_{\rm c}$ would be higher to be close to the `N\'{e}el temperature' of the Heisenberg model in Eq. (\ref{eq20}). This improvement is an interesting problem; however, in this paper, leaving this as a future problem, we treat pairing fluctuations within SCTA and discuss effects of CDW and SDW fluctuations in the next section.
\par

\begin{figure}
\includegraphics[scale=0.7]{fig6}
\caption{$T_{\rm c}$ as a function of the filling number $n$. The result within the SCTA and that within the NSR theory are compared. We set $U/6t=1$.
\label{fig6}
}
\end{figure}
\begin{figure}
\includegraphics[scale=0.7]{fig7}
\caption{Chemical potential $\mu$ at $T_{\rm c}$ calculated within the NSR theory.
\label{fig7}
}
\end{figure}
\par
Before ending this section, we briefly note that the NSR theory does not
satisfy the particle-hole symmetry, when it is applied to the Hubbard
model. As shown in Fig.\ref{fig6}, the calculated $T_{\rm c}$
based on the NSR theory is unphysical around $n=2$. (Note that the system
must be a band insulator at $n=2$, leading to vanishing $T_{\rm c}$.). We also find that the required symmetric filling dependence of $T_{\rm c}$ with respect to $n=1$ is not obtained within the NSR theory.
In addition, although the chemical potential must satisfy $\mu=-U/2$ at $n=1$ due to the particle-hole symmetry\cite{Valkov}, the NSR result satisfies it only in the BEC limit $U\to\infty$, as shown in Fig.\ref{fig7}. In contrast, in addition to the symmetric filling dependence of $T_{\rm c}$, SCTA can also reproduce the exact result $\mu=-U/2$ at $n=1$ over the entire BCS-BEC crossover. (See Fig.\ref{fig4}.) We emphasize that satisfying these required conditions is important in any consistent theory.
\par
\begin{figure}
\includegraphics[scale=0.7]{fig8}
\caption{Superfluid phase transition temperature $T_{\rm c}$ as a
 function of pairing interaction $U$ and filling number $n$. In this
 figure, and in Fig.\ref{fig9}, we include CDW and SDW fluctuations
 described by $\Sigma_{\rm ph}^{d,s}$ in addition to pairing
 fluctuations.
In comparison with Fig.\ref{fig4}, $T_{\rm c}$ around $n=1$ are suppressed in the strong coupling regime.
\label{fig8}
}
\end{figure}
\begin{figure}
\includegraphics[scale=0.7]{fig9}
\caption{Chemical potential $\mu$ as a function of $U$ at $T_{\rm
 c}$ when we consider CDW and SDW fluctuations in addition to pairing fluctuations. Self-consistent
 treatment of CDW and SDW fluctuations does not break the particle-hole symmetry
 condition $\mu=-U/2$ at $n=1$.
\label{fig9}
}
\end{figure}

\begin{figure}
\includegraphics[scale=0.7]{fig10}
\caption{Effects of CDW and SDW fluctuations on $T_{\rm c}$ at the half-filling $n=1$. SCTA: Pairing fluctuations are only included. SCTA+CDW+SDW: Pairing, CDW, and SDW fluctuations are all included. SCTA+CDW: Pairing and CDW fluctuations are taken into account. These abbreviations are also used in Figs.\ref{fig11} and \ref{fig12}.
\label{fig10}
}
\end{figure}

\begin{figure}
\includegraphics[scale=0.7]{fig11}
\caption{Denominator of the static charge susceptibility $\chi({\bf Q})$ in Eq. (\ref{eq12}) at the superfluid phase transition temperature $T_{\rm c}$. The CDW instability is determined when $1-U\Pi_{\rm ph}(\bm{q}=\bm{Q},\omega =0)=0$ is realized.
\label{fig11}
}
\end{figure}

\section{Effects of CDW and SDW fluctuations}

Figures \ref{fig8} and \ref{fig9} show calculated $T_{\rm c}$ and $\mu(T_{\rm c})$ respectively in the BCS-BEC crossover, when the CDW ($\Sigma_{\rm ph}^{\rm d}$) and SDW fluctuations ($\Sigma_{\rm ph}^{\rm s}$) are both taken into account. As shown in Fig. \ref{fig9}, the required condition $\mu=-U/2$ at $n=1$ is still satisfied when one includes CDW and SDW fluctuations within FLEX.
\par
Comparing Fig.\ref{fig4} with Fig.\ref{fig9}, one finds that effects of CDW and SDW fluctuations on the chemical potential $\mu$ are weak. In contrast, from the comparison of Fig.\ref{fig3} and Fig.\ref{fig8}, $T_{\rm c}$ is found to be suppressed near the half-filling when these fluctuations are taken into account.
\par
To see the suppression of $T_{\rm c}$ more clearly, we show $T_{\rm c}$ at $n=1$ in Fig.\ref{fig10}. At the half-filling, the CDW instability occurs simultaneously (which is confirmed by vanishing denominator of the charge susceptibility $\chi({\bf Q})$ as shown in Fig.\ref{fig11}), which leads to the remarkable suppression of $T_{\rm c}$. However, in contrast to the two-dimensional case, where $T_{\rm c}$ vanishes at $n=1$\cite{Scalettar}, we still obtain a finite $T_{\rm c}$ even at the half-filling.
\par
Although SDW fluctuations are weak in the attractive Hubbard model, we still find their effects around $U/6t\sim 1$ in Fig.\ref{fig10}. From the comparison of the result referred to as 'SCTA+CDW+SDW' with 'SCTA+CDW' in Fig.\ref{fig10}, we find that SDW fluctuations weaken the suppression of $T_{\rm c}$ by CDW fluctuations.
\par
In this intermediate coupling regime, since the binding energy of a Cooper pair is not very strong, (pseudo)spin degrees of freedom still remains, which contribute to SDW fluctuations. As one approaches the strong-coupling regime, these spin degrees from freedom disappear due to the formation of singlet pairs. Indeed, in Fig.\ref{fig10}, the two results, 'SCTA+CDW+SDW' and 'SCTA+CDW', give almost the same $T_{\rm c}$ when $U/6t\ \raise.3ex\hbox{$>$}\kern-0.8em\lower.7ex\hbox{$\sim$}\  3$.
\par
\begin{figure}
\includegraphics[scale=0.7]{fig12a}\\
\includegraphics[scale=0.7]{fig12b}\\
\caption{Filling dependence of the superfluid transition temperature $T_{\rm c}$. Upper and lower panels show the cases of the weak-coupling BCS regime ($U/6t=0.7$) and strong-coupling BEC regime ($U/6t=2$), respectively.
\label{fig12}
}
\end{figure}
\par
Although the degeneracy of the superfluid state and CDW is absent when
$n\ne 1$, we can still expect strong influence of CDW near the
half-filling due to strong enhancement of charge susceptibility shown in
Fig.\ref{fig11}. Indeed, as shown in Fig.\ref{fig12}, CDW fluctuations
suppress $T_{\rm c}$ near $n=1$. (Compare `SCTA' with `SCTA+CDW+SDW' in
Fig.\ref{fig12}.) The maximum $T_{\rm c}$ is thus obtained, not at the
half-filling, but away from the half-filling. Although SDW fluctuations
enhance $T_{\rm c}$, the overall behavior is unchanged. (Compare
`SCTA+CDW+SDW' with `SCTA+CDW' in Fig.\ref{fig12}.) Since spin degrees
of freedom are almost absent in the strong-coupling regime, effects of
SDW fluctuations are weaker in the lower panel (BEC regime) than the
upper panel (BCS$\sim$crossover regime) in Fig.\ref{fig12}.

\par
\par
\section{Summary}
To summarize, we have discussed the superfluid phase transition in the
BCS-BEC crossover regime of a two-component Fermi gas loaded on a
three-dimensional optical lattice. Treating this system as the
attractive Hubbard model, we calculated the superfluid phase transition
temperature $T_{\rm c}$, including pairing fluctuations within the
self-consistent $t$-matrix theory, as well as CDW and SDW fluctuations
within the fluctuation exchange approximation. We determined $T_{\rm c}$
and the Fermi chemical potential $\mu$ self-consistently as functions of
the pairing interaction $U$ and filling number $n$ in the BCS-BEC
crossover region, by solving the equation for $T_{\rm c}$, together with
the number equation.
\par
CDW fluctuations are strong near the half-filling due to the nesting
property of the Fermi surface at $n=1$. These strong fluctuations
remarkably decrease the superfluid phase transition temperature $T_{\rm
c}$ around $n=1$. As a result, the maximum $T_{\rm c}$ is obtained, not
at the half-filling, but away from the half-filling. We also showed
that, although SDW fluctuations are weak in the attractive Hubbard
model, they still affect $T_{\rm c}$ to increase slightly in the intermediate coupling region
$U/6t\sim 1$.
\par
We have also discussed the validity of SCTA.
Our theory satisfies the required condition associated with the particle-hole symmetry of the
Hubbard model which is not derived from NSR theory.
Therefore, it would be a good starting point to improve the BCS-BEC crossover theory in optical lattices.
On the other hand, we showed that this
approximation underestimates $T_{\rm c}$ in the BEC regime. As a key to
understand this, we pointed out the importance of a repulsive
interaction between molecules. Since the Gaussian fluctuation theory
(which completely ignores the molecular interaction at $T_{\rm c}$)
largely {\it overestimates} $T_{\rm c}$, we expect that SCTA
overestimates effects of the molecular interaction. Indeed, the
overestimate of the molecule interaction within SCTA has been pointed
out\cite{Haussmann94,Strinati,Petrov,Gio,Ohashi3} in a uniform Fermi gas
with no lattice potential. Inclusion of the correct value of the
molecular interaction in the present theory is our future
problem.
\par
So far, the superfluid Fermi gas in an optical lattice has been realized
when the lattice potential is weak\cite{chin06}. To really realize the
Hubbard model in a cold gas of Fermi atoms, stronger optical lattice
potentials must be used, which, however, inevitably leads to a small
nearest-neighbor hopping $t$, as well as low $T_{\rm c}$. Thus, to
realize Fermi superfluids in such a difficult situation, our results
indicate that the filling number should be set to be away from $n=1$ (to avoid the suppression of $T_{\rm
c}$ by CDW fluctuations) so that one can reach $T_{\rm c}$ as easy as
possible under a given experimental condition. Since the Hubbard model
is a fundamental model in condensed matter physics, realization of Fermi
superfluid in the Hubbard model produced by strong optical lattice
potential would be great challenge in cold atom physics.
\acknowledgments
This work was supported by a Grant-in-Aid for Scientific
Research of Priority Area ``Physics of New Quantum Phase in Superclean
Materials'' from the Ministry of Education, Culture, Sports, Science and
Technology of Japan (MEXT). The authors were also supported by MEXT
(No. 19340099 (H. T. and K. M.), and 19540420 (Y. O.)).

redpajama_set_name: RedPajamaArXiv


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text:
New program allows Franklin High School students to earn credit for Rutgers courses
Catherine Nguyen
Photo by Google Maps
Franklin High School, located in Somerset, New Jersey, will soon be allowing high school students interested in healthcare fields to take courses that translate to Rutgers credit. The program will select 24 students for its first year.
A new program presented Wednesday night will allow high school students from Franklin High School, located in Somerset, to earn 10 credits from Rutgers by the time they graduate, according to TAP Into.
At Franklin Middle School—Hamilton Street Campus, Eric Siegal, district supervisor of science at the school, introduced the program to a group of parents. Twenty-four students interested in working in the healthcare industry will be chosen for the program, and will take classes throughout high school that also counts as University credit. The initiative, considered a "health professions academy," aims to give students at Franklin a unique opportunity in all aspects of healthcare.
"Not all healthcare is delivered by doctors. If a student is interested in working as a lab tech, or medical assistant, or a nurse, or a phlebotomist who is someone who draws blood or maybe working in a psychiatric institution ... this would be a program that prepares students to major in those fields," Siegal said. "With the aging population we have in this country, there will be a lot of STEM jobs available to students to serve in a healthcare capacity that's not necessarily a doctor."
The program will start this September, with incoming first-years taking courses such as the Dynamics of Healthcare, Medical Terminology, Human Anatomy, Math in Medicine and Scientific Principles of Nutrition. High school teachers at the school will be accepted as adjunct faculty, with the curriculum being identical to classes offered at Rutgers. At the end of each class, these students will also take the same exam as the one given at the University for their respective classes.
"It's the same curriculum, same exam, but it's done at Franklin High School. These are official Rutgers credits and the grades will appear on a Rutgers transcript as if they had gone to Rutgers as an 18 or 19-year-old freshman," Siegal said.
He encouraged all students to apply, emphasizing to parents that it was not exclusively for the most high-achieving students.
"This is not an honors program. This is not selected for a few. We're looking for students at about a B-plus who have good behavior and good attendance," he said.
The selection process involves a board-approved rubric in which academic performance has an equal weight to personality. Siegal said this was because the program hopes to foster nurses and health practitioners who have empathy, so while students will be judged on grades, essays and letters of reference, they will also be judged by an interview.
The district will look at students' average grades over the span of three years in mathematics, science and English, as well as PARCC test scores, a letter of interest written by the student and an in-person interview to select the first group of students in the program. All of the requirements will take place while students are in school, including the interview and written letter of interest.
Rutgers will require these students to take certain prerequisites, such as biology for first-years and Algebra I. In the case that a student wants to take a different science class, such as AP Physics, Siegal said they would be accommodated on a case-by-case basis.
To stay in the program, students must maintain a 74% average for courses in the program, and an 80% in their classes overall. They are also required to complete 10 hours of clinical experience.
"It could be going to the doctor's office with a relative or witnessing or participating in physical therapy," Siegal said. "Anything relating to a health profession. It's a very large umbrella of activities that are approved."
Siegal also assured parents that these students would also have time for other extracurriculars.
"They can still do sports, they can still do after-school activities, they still take the same bus. The only difference is for certain courses throughout their four years, they'll be taking courses together as the 24-person cohort," he said.
The program is also much cheaper for these students than what it would normally cost. Ten nursing credits at Rutgers would cost approximately $4,630, but the exam fees for the high school students in the program add up to $140.
While the program only limits students to gain 10 credits, the district hopes to increase that amount to a maximum of 34 credits.


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Take One Last Look! NY Yankees' Legend's Mansion to Be Demolished [PHOTOS]
Dan Bahl
Dan Bahl Updated: September 23, 2022
Getty Images / Realtor.com
Derek Jeter made roughly $265 million in salary alone during his baseball career. So, naturally, he can afford some fairly luxurious things in his post-playing days.
One such item of luxury was a luxury mansion in Florida, which Jeter bought in 2012 for $15.5 million, according to a story done by The New York Post. Jeter has since sold the property, and now, it appears as though the house's days may be numbered.
The story by the Post asserts that the house, which was owned by New York Yankees' legend Derek Jeter from 2012 through May of 2021, is set to be demolished. The story explains that a demolition application had been taken out for the house, with the ultimate goal being to use the expensive real estate for commercial purposes moving forward.
We found photos of the house on Realtor.com, and boy, it would be a real shame if this house did end up getting taken down.
Before we show you photos from inside and outside the house, a quick note on its history. In 2020, the luxury mansion welcomed new tenants, as Jeter rented his Tampa home to Tom Brady and his wife, Gisele Bündchen, along with the rest of the Brady family. Brady and Co. called the property home during his first year with the Tampa Bay Buccaneers, as the family re-located from their long-time residence in New England.
Brady would end up leaving the home, citing a lack of privacy as the main reason for choosing to re-locate elsewhere.
It was soon after the Brady bunch's departure that Jeter would put the home on the market, selling it for $22.5 million in 2021. Less than one year later, in February of 2022, Jeter would cut ties with his other major connection to Florida, selling his 4% ownership of Major League Baseball's Miami Marlins.
Now, to the house itself. It's a six-bed, 5.5+ bath, 4,500 square-foot castle of a home, which sits directly on the shores of the beautiful Hillsborough Bay. With real estate prices skyrocketing, the value of the house eclipsed the $30 million mark of August of this year.
Despite that, the demolition appears destined to begin soo. Take one final look inside Derek Jeter's former home, before it's possibly reduced to rubble in the coming months.
New York Yankees' Legend's Beautiful Mansion to Be Demolished [PHOTOS]
Did Tom Brady ruin something else in New York sports? We're not sure, but a Derek Jeter-owned mansion that was rented by Brady is being demolished soon. Take a look inside below.
NY Yankee Legend's Former House For Sale! What's It Look Like Now?
The former house of a New York Yankees' legend is back on the market in New Rochelle, New York. Take a look inside and see what it looks like in present-day.
Source: Take One Last Look! NY Yankees' Legend's Mansion to Be Demolished [PHOTOS]
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Comparison of Radiation Protocols for Pre-pectoral vs. Sub-pectoral Implant-based Breast Reconstruction
Libby R. Copeland-Halperin, MD, Yulia Lyatskaya, Ph.D, Jennifer R. Bellon, MD, Matthew J. Carty, MD, Jessica Erdmann-Sager, MD.
The Brigham and Women's Hospital, Boston, MA, USA.
PURPOSE: In the United States, approximately one third of patients who undergo mastectomy will undergo post-mastectomy radiation therapy (PMRT). The presence of breast reconstruction may alter how PMRT is delivered. Pre-pectoral implant-based reconstruction has been widely adopted, but there is no data on the impact of pre-pectoral implant-based reconstruction on PMRT planning or delivery. Rather, prior studies have focused on complication rates and aesthetic outcomes. This study aims to examine whether there is a difference in radiation administration among patients undergoing pre-pectoral and sub-pectoral implant-based reconstruction.
METHODS: Radiation mapping protocols for 50 patients who received either immediate sub-pectoral or pre-pectoral implant-based reconstruction followed by PMRT at a large academic medical center will be retrospectively reviewed. The main outcomes of interest are whether patients who underwent pre-pectoral reconstruction have an increase in focal areas of decreased radiation delivery (i.e. "cold spots") in the pectoralis major muscle, and/or whether they have an increase in unwanted radiation reaching the heart and lungs.
RESULTS: The radiation protocols for 25 patients undergoing pre-pectoral and 25 undergoing sub-pectoral reconstruction followed by PMRT will be reviewed.
CONCLUSION: As pre-pectoral implant-based breast reconstruction becomes more common, it is essential to further study the effects of this technique on radiation dosing and oncologic outcomes. This is an initial exploratory study. Larger prospective studies are needed to better analyze long-term effects of pre-pectoral implant-based reconstruction on radiation dosing and recurrence rates.