text:
Americans & Veterans Against Jihad
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Ebola : Inside the Deadly Outbreak (Documentary 2014)
Posted on October 16, 2014 by avaj1492
OUTBREAK!
Ebola: Political correctness could kill a lot of us
Pat Buchanan: Community and country come ahead of any
obligation to people of Africa
Growing up in Washington in the 1930s and '40s, our home was, several times, put under quarantine. A poster would be tacked on the door indicating the presence within of a contagious disease – measles, mumps, chicken pox, scarlet fever.
None of us believed we were victims of some sort of invidious discrimination against large Catholic families. It was a given that public health authorities were trying to contain the spread of a disease threatening the health of children.
Out came the Monopoly board.
Polio, or infantile paralysis, was the most fearsome of those diseases. The first two national Boy Scout jamborees, which were to be held in Washington in 1935 and 1936, were canceled by presidential proclamation because of an outbreak of polio in the city.
Franklin Roosevelt, who had apparently contracted polio in 1921, never to walk again, appreciated the danger. In the 1930s, '40s and early '50s, there were outbreaks of polio in D.C. Swimming pools were shut down.
The Greatest Generation possessed a common sense that seems lacking today.
We read that five new Ebola cases occur every hour in Liberia, Guinea and Sierra Leone, that thousands are dead and thousands more are dying, that by December, there may be 10,000 new cases a week of this dreadful and deadly disease.
Yet calls for the cancellation of commercial airline travel from the affected nations to the United States are being decried as racist, an abandonment of America's responsibilities to Africa, a threat to the economies of the poorest continent on earth.
How could we consider such a thing!
Where once we suffered from infantile paralysis, now we suffer from ideological paralysis. And there appears to be no Salk or Sabin vaccine to cure our condition.
Exhibit A is the befuddled response of some in public service is the case of Amber Joy Vinson.
Nurse Vinson was among 75 health-care providers who treated Thomas Eric Duncan, the Liberian who brought Ebola into the United States. At the Texas Health Presbyterian Hospital where Duncan was treated, Vinson had been among those in closest contact with the patient.
Two days after Duncan's death, Vinson was allowed to fly to Cleveland to visit relatives. She then prepared to fly back to Dallas.
Before boarding, she called the Centerd for Disease Control and said she was running a fever of 99.5. Yet she was given clearance to fly commercial back to Dallas, where she was admitted to the hospital with symptoms of the disease. She is the second nurse at that hospital to come down with Ebola.
According to CBS Medical Correspondent Dr. John LaPook, "Nurse Vinson did in fact call the CDC several times before taking that flight and said she had a temperature, a fever of 99.5, and the person at the CDC looked at a chart, and because her temperature wasn't 100.4 or higher she didn't officially fall into the category of high risk."
Would not common sense have told that CDC apparatchik to tell Vinson not to fly at all, but remain in Cleveland, stay in touch with CDC and monitor any symptoms to be sure she was not coming down with the disease that just killed her patient?
In dealing with contagious and deadly diseases, common sense says to err on the side of safety. Public safety must come before political correctness. Community and country come ahead of any obligation to the people of West Africa.
Indeed, is not the first duty of the government of the United States to protect the lives, liberty and property of the citizens of the United States?
Traveling to Africa decades ago, Americans were given a series of shots to avoid contracting indigenous diseases. Travelers to the United States were questioned about diseases to which they may have been exposed in Third World countries.
Now we have a government that considers it discriminatory to put troops on our frontiers to halt the invading millions from across the Mexican border, and the mark of a cruel and cold people to send back lawbreakers who have broken into our country.
The two nurses who came down with this disease after close contract with Duncan are being cared for in quarantine, as is the NBC crew, one of whom contracted the disease. And rightly so.
As for U.S. aid workers in Africa, they are heroic. But before bringing these good and brave people home, we ought to be sure they are not bringing back with them the Ebola they have been fighting.
If that means quarantining them for 21 days, so be it. If that means no commercial flights to the United States from the three most affected countries of West Africa, and no admission to the USA of any travelers whose visas show they have been in those countries in recent days, then it ought to be done.
Otherwise political correctness is going to end up killing a lot of us.
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In this fourth issue of our blog we look at wurstscript's start into 2018, and our roadmap. Once again we're excited to mention that users within our awesome community are getting involved and contribute to the wurst.
The runmap command now uses war3.exe if it is present, which can improve loading time. The game executable detection has also been improved.
Compiletime mocks added for force and gamecache, enabling them to be ued in object editing and unit tests.
Special thanks to @Sir Moriarty for providing us with new and improved FileIO and Sync packages. The biggest PR we have merged so far!
Wurst's underlying mpq library JMPQ has been updated to support pkware decompression and file-less data extraction.
The Wc3libs have been updated as well, providing WTS support and Jass's StringHash implementation.
Note: The showcase is now official - you should submit your wurst maps for a chance in the spotlight!
Preamble: The 'unit' in unit testing does not refer to wc3 units - rather, a unit is an individual piece of source code that is being tested.
One of the caveats of unit testing is that compiletime jass interpretation depends on the completeness and correctness of the wurst compiler that is performing the testing instead of the warcraft engine. Wurst does not implement every native, and since we don't know the inner workings of wc3, it can't emulate everything identically.
Prove that your code does what it's supposed to do.
The easiest units to test are the ones that don't include warcraft specific elements. Here are some condensed example unit tests for our data structures, arithmetics and string manipulation from the standard library.
To make any function a test, just annotate it with @Test. All functions with this annotation will then be recognized by wurst. This doesn't limit the function in any way and it could theoretically still be used inside your code and not exclusivly as test, however that is not recommended.
A unit test consists of two parts - the execution of the to be tested code and an assertion, that compares the actual result with an expected value. You can find the assert functions inside the Wurstunit package.
In VScode, use F1 to open the task prompt and enter "run test" and choose one of the options.
And that's it! You are now a testing guru. We hope you enjoyed reading this, and we look forward to next month's blog post wherein we'll take a practical look at composing visually beautiful spells in wurst.


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In today's Gospel Reading there is an incident that is unique. Jesus did something that no one before him had done. He put two commandments together, now known as "The Summary of the Law." We heard this near the beginning of our Eucharist this morning, just before the Confession. This incident is also unique because both the scribe and Jesus dealt throughout the whole event in a friendly way.
It is by this Summary of the Law that we can love God by loving our neighbor, as well as loving God directly.
This freedom to love God in many ways, by our love and respect shown to one another, and by showing our love to God directly, is affirmed in the 1st letter of John.
(1 Jn 4:19) Think about it and pray with it!


Life is short. Be a Mermaid!
Our 7 day program will entail gentle introduction to meditation and yoga practice to suit the group. Awakening and deepening our connection to body through movement and breath. In our stillness, allowing space for "spirit" to flow in and guide us to our higher purpose and path.
Our adventure activities are designed to enhance and inspire our personal and spiritual growth. Snorkelling to explore reef and discover marine life, sailing with the wind as our fuel, yoga with the sand between our toes, fresh tropical fruits, warming sunshine, and lush rainforest to feed us fresh oxygen and keep us grounded on this adventure of a lifetime.
Be a part of a committed group of women to support each other to our most vibrant experience of health, our greatest experiences of joy, and to live our most impactful life yet. There are very limited spots available. We do this to foster greater connection in the group and support the journey of each individual.
We will be playing in the ocean and in nature, to connect to our childlike selves, finding immense joy, wonder, and awe as we explore and discover. Fostering deep gratitude, which is the foundation of our transformation.
Discover leadership skills from environmental activists and politicians, and soak in local wisdom with an indigenous community. Awaken your higher self and your greater purpose through daily yoga and meditation to strengthen and heal mind, body and spirit. Honour the divine feminine within us through ritual and ceremony.
Join me in Western Australia for a magical week of yoga, meditation, swimming with whale sharks in the incredibly biodiverse Ningaloo Reef, a special plastic pollution campaign, and practicing a plastic free lifestyle.
The whales are migrating south with their freshly born calves. Come along to interact non-invasively and connect with the gorgeous new families.
Kate Nelson's golden edge is to integrate fluid mermaid magic in with the environmental movement, reinventing conservation and aiding the collective shift through positive energy and luxury adventure. Kate feels called here in this lifetime to support the awakening of women leaders while helping them achieve even greater outcomes for their purpose, their community, and the planet.
Kate strives for mass global shift through feminine, fluid empowered PLAY. By releasing into childlike joy through adventure and "mermaiding" she opens hearts and minds to a new way of being. She has taught over 1 million people the skills to let go of the synthetic way of life, products, and relationships to return back to the organic and natural. Having led transformational adventures to exotic locations for women from all over the world and different backgrounds, she is consistent in her results. Creating powerful, lasting change in participants and leaving the visited location better than she found it. The Give Back Program is now over a decade old. Under this program Kate has worked along California legislators on the successful plastic bag ban campaign in California, she has sat on the board of Advisors to the Australian Minister of the Environment, worked on plastic pollution campaigns for GreenPeace, San Diego Coastkeeper, Surfrider Foundation, and founded the non-profit organisation Save the Mermaids in 2009.


text:
Helge Pedersen (born c. 1955) is a long-distance motorcyclist originally from Kristiansand, Norway, who now resides in Seattle, Washington. He traveled more than  touring the world on a BMW R80G/S adventure touring motorcycle between 1982 and 1992. This journey is recounted in his book 10 Years on 2 Wheels. The motorcycle he rode on was placed on display at the BMW Museum in Munich.

Pedersen has been "prominent in the motorcycle industry", continuing to ride and lead tours since 1993. For example, he led three  trips to Tierra del Fuego by 2013.

He started a motorcycle touring company in his city of residence, Seattle in 1998, and has published a series of instructional and adventure documentary DVDs.

Bibliography/filmography

GlobeRiders documentary DVD series
Africa Adventure  (2011)
Eurasian Odyssey  (2009)
IndoChina Expedition  (2008)
Silk Road Adventure  (2007)
Iceland Expedition  (2006)
GlobeRiders instructional DVD series: BMW F800GS Adventure Touring Instructional DVD, BMW R1200GS Adventure Touring Instructional DVD, BMW R1100GS/1150GS Adventure Touring Instructional DVD, BMW F650GS Adventure Touring Instructional DVD

References

Further reading

BMW R1200GS Adventure build, Ultimate Motorcycling

Long-distance motorcycle riders
Businesspeople from Seattle
Writers from Seattle
American travel writers
American male non-fiction writers
American documentary filmmakers
Motorcycle tour guides
Motorcycle touring writers
1950s births
Living people
People from Kristiansand
Norwegian emigrants to the United States

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This episode is sponsored by Soft Skull, Counterpoint, and Catapult. Special thanks to Joe and Stephanie Douglas, Big Hair Studios, Allen Watke, Phil Heaven and the Midnight Mystery Players, and George Kaas for the equipment loan that made this recording possible. And of course thanks to Sam Kaas (who longtime listeners may recognize from Episode 7) our production manager without whom this whole episode would not have been amplified, recorded, nor kept on track.
Emma is really into female rage right now, nbd.
also mentioned, And Now We Have Everything: On Motherhood Before I Was Ready by Meaghan O'Connell because (spoiler alert) we interview both authors later in the episode!
King's Books has fourteen book clubs, including one that only reads books about cults and one that only reads books about medical issues. They also have such unconventional events as virtual reality film showings and 80s workout nights (#Cher).
"being a bookstore owner and event planner and bookkeeper and etc... that I don't have a lot of time to read"
Uh, can all the booksellers whose "confession" this is raise their hands?
"a woman falls in love with a frog man; [he] shows up at her door... and she takes him in, in all the ways"
We are impressed by Ariana's practicality and thus let her, and the audience, in on our secret post-apocalypse library.
Fun fact, Waucoma Bookstore is only about 20 miles away from the Pacific Crest Trail where Cheryl Strayed ended her Wild trip.
Emma tweets from @thebibliot and is working on a newsletter where she writes about books. Kim occasionally tweets from @finaleofseem, but not enough to justify you bothering to follow her.


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Democrats Have So Far Failed To Flip A Single State Legislative Chamber, And Lost Two
Democrats have so far failed to flip any state legislative chambers and have already lost both in New Hampshire as votes from 2020's election continue being counted.
Heading into Tuesday, Republicans controlled 58 of 98 chambers, not including Nebraska's unicameral nonpartisan legislature. While that tally is down from the 65 controlled by the GOP headed into 2018 and the 68 before 2016, Democrats had hoped to make even more gains at the state level by running down-ballot against President Donald Trump.
"Democrats had targeted 10 legislative chambers they hoped to flip, and national groups raised at least $88 million to support that cause, compared with more than $60 million for Republicans," The Wall Street Journal reported. "The results mirror a weak showing for Democrats in U.S. Congressional races."
Significantly, Republicans in Texas fought off what the Texas Tribune called a "well-financed Democratic effort" to flip the Texas House. For their efforts, the balance will reportedly remain close to the 83-67 GOP majority it was last term.
Cook Political Report in October included 14 GOP held legislatures of its 19 "vulnerable chambers" and wrote that Democrats were "well-positioned to net up to a half-dozen new chambers this fall.
"Among the chambers still rated as Toss Ups, the Republicans hold all six: the Arizona Senate, the Iowa House, the Michigan House, the Minnesota Senate, the North Carolina Senate, and the Pennsylvania House," wrote Cook Political Report, which had also listed New Hampshire's legislative bodies as "lean Democratic."
So far, none of those have flipped to Democrats, and while control of Arizona's state bodies is still up in the air pending a final count, both New Hampshire's House and Senate are now controlled by Republicans, WSJ reported. The New Hampshire state Senate flipped from 14-10 Democratic to 14-10 GOP, while Republican candidates won dozens of races to gain control of the 400 member state House.
New Hampshire Republicans ran as a unified ticket that put New Hampshire first, and the result is an incoming Republican Majority in the Executive Council and both chambers at the State House. (1/2)
— Chris Sununu (@ChrisSununu) November 4, 2020
Control of statehouses not only affects state legislation, but also Congressional redistricting. The National Conference of State Legislatures told The Wall Street Journal that 24 of the 36 states where legislatures draw the district lines are now controlled by Republicans.
Previous articleMilitary ballots still arriving in swing states where vote count is unfinished
Next articleDem 'Squad' congratulate Biden, Harris: Now we can pursue 'the most progressive agenda' in US history

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Designed for District and Building Administrators, District and School Librarians, Technology Leaders, and Curriculum/Instruction Leaders.
This course will increase awareness of the impact that an effective library program can have on the school's culture of learning and will provide a practical framework for identifying specific strategies for school library improvement to support a district's mission and vision. Participants will use Linking for Learning: The Illinois School Library Standards, 4th edition, to complete a self-assessment of their leadership role and develop an action plan to impact student learning through the school library. This application component aligns with Illinois Professional School Leader Standard 1: Facilitating a Vision of Learning.
Participants not needing AA credit may opt to take the workshop for PDUs.


text:
Written by J Rohnny• December 18, 2022• 3:45 am• Europe Economy
How is Europe handling inflation, energy prices? | Opinion
As a proud Scot who has had the privilege of serving in both the House of Commons and the Scottish Parliament, I felt somewhat obliged to respond to the article written by Evan Ward titled "What the U.S. can learn from a recession in Britain." This article was overly negative and does not present, I believe, an accurate representation of what is happening in the United Kingdom.
Like most countries in the western world, the United Kingdom is facing a difficult economic outlook. Inflation is high as activity returns to the economy after two years of COVID-19 lockdown. Energy prices are rising due to economic sanctions against President Vladimir Putin's regime. These difficulties, however, are not unique to the United Kingdom, and it is disingenuous to suggest so.
Despite the political turmoil we have faced, the U.K. government has been nimble in its response to these challenges. The U.K. was the first country in the world, for example, to send defensive weapons to our friends in Ukraine, showing that we are willing to use our Brexit freedoms to defend liberty across the world, in spite of the economic consequences. Defending freedom often comes as an economic cost. It has in this instance.
The Energy Price Guarantee puts a cap on the amount you can be charged per unit of gas or electricity, to a household average of around £2,500 a year. This is saving individuals, families and businesses around £900 a year.
The U.K. government is taking proactive action to boost domestic energy supply, ensuring that our country becomes energy resilient and has much to teach the world on our approach. A new oil and gas licensing round has been launched, which is expected to lead to over 100 new licenses. There has been an acceleration of new sources of energy, including nuclear, wind and solar. The U.K. government is undertaking reforms to the structure and regulation of the U.K. energy market, making sure that this market serves the people's and country's needs.
In the three months prior to August 2022, U.K. exports increased by £6.8 billion. An example of an industry that is doing well, despite the difficult economic outlook, is Scotch whisky. During 2021, the value of Scotch whisky exports was up 19%. Growth was driven in Asia Pacific and Latin America, with strong growth also seen in India and Brazil. Despite Brexit, exports to the European Union grew by 8%. And using our Brexit freedoms, the U.K. government successfully negotiated the removal of the 25% tariff on Scotch whisky in the U.S., resulting in exports growing there as well.
It is not only trade that shows signs of encouragement for the U.K. economy. A report from Dealroom shows that London has attracted £7.8 billion in fintech venture capital funding since the start of 2022, edging it ahead of both San Francisco and New York to become the world's biggest center for fintech investment. The Z/Yen group's latest green finance index, released in October, showed that London is the greenest financial center in the world.
These success stories show that the U.K. is embracing economic innovation, understanding that this is a central ingredient to growth. Liz Truss was also right to emphasize the need for supply-side reform, and we are seeing a lot of her arguments in this field being implemented by the government led by Rishi Sunak.
What has impressed me the most about my country in the past six months, however, is how calm our citizens have been. Having three Prime Ministers and a new monarch, after the longest ever reigning monarch in British history, could have caused disarray. Yet, as the saying goes, the British kept calm and carried on. It is who we are and what we expect of ourselves after centuries of doing things in our own peculiar way.
With poignancy, Britain was on the world stage in September after the death of Her Late Majesty, Queen Elizabeth II. On the drive from Balmoral to Edinburgh, Scotland's natural beauty was on display. The funeral in London and Windsor showed the power of Britain's customs and traditions. And throughout all of this, the people of my country were united.
It is in this promotion of the common good that the British spirit remains high; that we continue to push above our weight when things appear to be difficult; and it is why we will take full advantage of our newfound freedoms and forge closer ties with one of our greatest allies, the United States of America.
Stephen Kerr is a member of the Scottish Parliament and a former member of the United Kingdom Parliament.
Future of cryptocurrency
Crypto Week At A Glance: Bitcoin drops below $17K as US Fed remains hawkish


text:
Q: What is the error in this MS-DOS bit? I'm making a DOS game, and the first thing to come up is the option to play the game or learn to play the game.  This is the code bit I believe is being weird:
SET /P startgame=Selection:
if %startgame%=="how2play" goto how2play
if %startgame%=="play" goto play
if %startgame%=="" goto launch
goto codeerror

Here are the intended actions:
SET: User input of "play" or "how2play" it set to variable "startgame"
IF: "startgame" variable used to redirect user to "how2play" or "play"
Here is what happens instead:
Rather than havinng the intended outcome of either option, it goes straight to the failsafe, being "codeerror"
Notes:
In this bit, I did not include the "codeerror", "how2play", or "play" bits in this question, but if they are necessary to find an answer as to why the IF statements (I suppose) are not working, let me know.  "launch" is also included in this bit, however this code bit is part of the "launch" operation, the only thing missing from it is some text just printed onto the console using the "echo" command.

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In addition to being selected as one of 50 scholars awarded fellowships each year at the prestigious Radcliffe Institute at Harvard University, the UA's Feryal Ozel has won the 2013 American Physical Society's Maria Goeppert Mayer Award for her cutting-edge research on neutron stars.
Feryal Ozel studies two things most people don't think about everyday: neutron stars and black holes.
An associate professor of astronomy at the University of Arizona, Ozel has won the 2013 American Physical Society's Maria Goeppert Mayer Award for her work on neutron stars and her dedication to public outreach and education in science and astronomy. In addition, this year she is completing a prestigious fellowship at the Radcliffe Institute at Harvard University. Ozel came to the UA in 2003 as a NASA Hubble fellow and began a faculty position in 2005.
Neutron stars are super energetic dense remnants of collapsed stars comprised primarily of subatomic particles called neutrons. According to some calculations, the average size of a neutron star is around 12 kilometers, or 7.5 miles, even though it can pack about 1.5 times the mass of our sun.
Ozel is investigating ways to more precisely measure the size of these solar relics, either by analyzing the spectrum of light waves that they emit, or by measuring and modeling the periodic variation of signals from neutron stars, which rotate around their own axes like a spinning top.
"This happens naturally on neutron stars where one side becomes brighter than the other. Part of the surface is hotter than the rest, and when it's hotter, it's brighter. We see the variation in brightness in stars that spin about their axis as an on-off signal," Ozel said, as though someone were switching the light on and off.
"We can measure how big they are based on this periodic variation in brightness." Astronomers can further use the variation in light to make a map of neutron stars' surfaces.
Ozel's second project focuses on black holes, preparing for an event that could change how we understand what are perhaps the universe's most mysterious entities: super-massive invisible objects that absorb anything that draws near to them, even light.
Ozel's "something" is a cloud, most likely comprised of hydrogen gas, about three times the size of the Earth and heading toward the black hole at the center of our own galaxy at considerable speed.
It will arrive there sometime around July, providing astronomers a chance to observe the result of the impact of the cloud with the black hole.
The cloud is moving fast enough through space that Ozel and her colleagues predict it will create a shockwave in front of it when it approaches the black hole, like the supersonic boom heard when an airplane breaks the sound barrier, Ozel said. The shockwave should emit radiation observable through radio telescopes.
"Shortly after that we expect that the cloud is going to be basically wrenched apart," Ozel said.
Astronomers can infer that the intense gravity of black holes absorbs material from objects that come too near, Ozel said, but normally aren't able to see it happen in real time. The collision of the gas cloud with the black hole at the center of our own galaxy will give scientists a chance to learn about the environment of a black hole.
"It's the first time we will be able to see a black hole having lunch," Ozel said.
Ozel's work involves developing computational models using known physics to predict what the environment around black holes could be like, or what the surface of a neutron star should look like.
"That is the forward approach," Ozel said. "The backward approach is to look at the data" and make inferences about these mysterious objects from what has been seen in observational studies. "I love doing both," she added.
Ozel will conclude her fellowship at Radcliffe Institute after the 2012-13 year and return to the UA.


Metasploit has a nifty PHP Remote File Include module that allows you to get a command shell from a RFI.
SRVHOST 0.0.0.0 yes The local host to listen on.
SRVPORT 8080 yes The local port to listen on.
[*] PHP include server started.
Knew there was a nicer way to do that then going through the pain of manually generating the exploit, throwing it on a server, and starting the payload handler, but I couldn't remember where it was at. That had been bothering me. Thanks!
I didn't see anything in the options for setting cookies so looks like this is for unauthenticated vectors only.
I hope this gets added.
good point. submit a ticket on msf site and im sure it will get added.


We have an exciting opportunity for an enthusiastic and experienced Receptionist to support legal secretaries in an international legal firm based in the City of London.
We are looking for a polished, personable and dynamic Receptionist as soon as possible, as this is a role that won't be around for long.
* Switchboard - answering calls, taking messages, etc.
* Permanent member of the Social Committee which includes arranging month-end drinks and purchasing all food and drinks, plus the organisation of two annual events.
Basic mark-ups and basic secretarial duties, i.e. printing, photocopying, scanning, etc.
Amazing salary and benefits include: private medical, pension and competitive holidays.


text:
Q: Why am I getting a SyntaxError when instantiating a __repr__method I receive the following error when I instantiate a class with a repr method I have.
When I remove the repr it works fine:
repr removed
class Wide():
    def __init__(self,  XfromLeftEdge = 141.0, YfromTopEdge = 300.0, Width = 1551.0, Height = 800.0 ):
        self.XfromLeftEdge =XfromLeftEdge
        self.YfromTopEdge =YfromTopEdge
        self.Width = Width
        self.Height = Height

    def objOne(self): #XfromLeftEdge, YfromTopEdge, Width, Height
        return XfromLeftEdge, YfromTopEdge, Width, Height

a = Wide()
print(a)

return:
<__main__.Wide object at 0x7faec1ed48b0>
(base) user SDNrig 6 %

with repr
class Wide():
    def __init__(self,  XfromLeftEdge = 141.0, YfromTopEdge = 300.0, Width = 1551.0, Height = 800.0 ):
        self.XfromLeftEdge =XfromLeftEdge
        self.YfromTopEdge =YfromTopEdge
        self.Width = Width
        self.Height = Height

    def objOne(self): #XfromLeftEdge, YfromTopEdge, Width, Height
        return XfromLeftEdge, YfromTopEdge, Width, Height

    def __repr__(self):
        return '{}, {}, {}, {}'.format(self.XfromLeftEdge = XfromLeftEdge, self.YfromTopEdge = YfromTopEdge, self.Width = Width, self.Height = Height)

    def __str__(self):
        return 'instance object of wide ROI object, XfromLeftEdge:{}, YfromTopEdge: {}, Width: {}, Height: {}'.format(
            self.XfromLeftEdge = XfromLeftEdge,
            self.YfromTopEdge = YfromTopEdge,
            self.Width = Width,
            self.Height = Height)

a = Wide()
print(a)

return
(base) user SDNrig 6 % /usr/local/bin/python3 "/Users/.../Desktop/SDNrig 6/play_f.py"
  File "/Users/.../Desktop/SDNrig 6/play_f.py", line 15
    return '{}, {}, {}, {}'.format(self.XfromLeftEdge = XfromLeftEdge, self.YfromTopEdge = YfromTopEdge, self.Width = Width, self.Height = Height)
                                   ^
SyntaxError: expression cannot contain assignment, perhaps you meant "=="?

Desired output
I would like to see print(a) give the params and their values.

A: You don't need the assignment in your format string.
Use this:
class Wide():
def __init__(self,  XfromLeftEdge = 141.0, YfromTopEdge = 300.0, Width = 1551.0, Height = 800.0 ):
    self.XfromLeftEdge =XfromLeftEdge
    self.YfromTopEdge =YfromTopEdge
    self.Width = Width
    self.Height = Height

def objOne(self): #XfromLeftEdge, YfromTopEdge, Width, Height
    return XfromLeftEdge, YfromTopEdge, Width, Height

def __repr__(self):
    return f"Wide({self.XfromLeftEdge}, {self.YfromTopEdge}, {self.Width}, {self.Height})"

def __str__(self):
    return f'instance object of wide ROI object, XfromLeftEdge:{self.XfromLeftEdge}, YfromTopEdge: {self.YfromTopEdge}, Width: {self.Width}, Height: {Self.Height}'

This will also use f-string syntax for more readability

A: This code will solve your error
class Wide():
    def __init__(self,  XfromLeftEdge = 141.0, YfromTopEdge = 300.0, Width = 1551.0, Height = 800.0 ):
        self.XfromLeftEdge =XfromLeftEdge
        self.YfromTopEdge =YfromTopEdge
        self.Width = Width
        self.Height = Height

    def objOne(self): #XfromLeftEdge, YfromTopEdge, Width, Height
        return XfromLeftEdge, YfromTopEdge, Width, Height

    def __repr__(self):
        return '{}, {}, {}, {}'.format(self.XfromLeftEdg, self.YfromTopEdge, self.Width, self.Height)

    def __str__(self):
        return 'instance object of wide ROI object, XfromLeftEdge:{}, YfromTopEdge: {}, Width: {}, Height: {}'.format(
            self.XfromLeftEdge,
            self.YfromTopEdge,
            self.Width,
            self.Height)

a = Wide()
print(a)

Or
class Wide():
    def __init__(self,  XfromLeftEdge = 141.0, YfromTopEdge = 300.0, Width = 1551.0, Height = 800.0 ):
        self.XfromLeftEdge =XfromLeftEdge
        self.YfromTopEdge =YfromTopEdge
        self.Width = Width
        self.Height = Height

    def objOne(self): #XfromLeftEdge, YfromTopEdge, Width, Height
        return XfromLeftEdge, YfromTopEdge, Width, Height

    def __repr__(self):
        return '{XfromLeftEdg}, {YfromTopEdge}, {Width}, {Height}'.format(XfromLeftEdg = self.XfromLeftEdg, YfromTopEdge =self.YfromTopEdge, Width = self.Width, Height =self.Height)

    def __str__(self):
        return 'instance object of wide ROI object, XfromLeftEdge:{XfromLeftEdge}, YfromTopEdge: {YfromTopEdge}, Width: {Width}, Height: {Height}'.format(
            XfromLeftEdge = self.XfromLeftEdge,
            YfromTopEdge = self.YfromTopEdge,
            Width = self.Width,
            Height = self.Height)

a = Wide()
print(a)

The problem was that in the string of the repr and str methods there is {} without a key and inside the format method, there is a key-value pair.
And the direction of the key and value was swapped.


This is a stub entry only — it provides links to other resources by and about Nick Bowd held in our catalogue.
Random Audio Sample: Back to the ranch : George W's farewell dance by Paul Cutlan, from the CD Selected Works by AMC Represented Artists, vol. 28.


text:
\section{Introduction}
Chern-Simons gravities (CSG) derived from non-Abelian Chern-Simons (CS) densities in $2+1$ dimensions were proposed by Witten in
Ref.~\cite{Witten:1988hc} and they were extended to all odd dimensions by Chamseddine in Refs.~\cite{Chamseddine:1989nu,Chamseddine:1990gk}.
CSG models consist of superpositions of gravitational models of all possible higher order gravities
in the given dimensions, each appearing with a precise
real numerical coefficient resulting from the calculus. In this report we refer to these models, aka. Lovelock models,
as $p$-Einstein gravities, the number $p$ being the power of the Riemann curvature in the Lagrangian, with $p=0$ being the
cosmological constant.

The recent work \cite{Tchrakian:2017fdw} has proposed
 a new formulation  of the CSG systems,
which allows their construction in all, $both$ odd and even dimensions. The derivation
of the new-CS densities follows exactly the same method as the $usual$-CS densities in odd dimensions. The $usual$ CS density results
from the one-step descent of the corresponding Chern-Pontryagin (CP) density.
The CP density being a total-divergence
\[
\Om_{\rm CP}=\pa_i\Om_i\ ,\quad i=\mu,D\ ;\ \quad\mu=1,2,\dots,d\ ;\ d=D-1\ ,
\]
the CS density is defined as the $D$-th component of $\Om_M$, namely $\Om_{\rm CS}\stackrel{\rm def.}=\Om_D$.

In the new formulation,
the role of the usual-CP density, which is defined in even dimensions only, is played by what we refer to as the
Higgs--Chern-Pontryagin (HCP) density, described in Refs.~\cite{Tchrakian:2010ar,Radu:2011zy} and in Appendix A of Ref.~\cite{Tchrakian:2015pka}.
These are dimensional descendents of the $n$th CP density in $N=2n$ dimensions, down to residual $D$ dimensions ($D<N=2n$), where now $D$
can be either odd or even. The relics of the gauge connection on the co-dimension are Higgs scalars. The remarkable property of the
HCP density $\Om_{\rm HCP}[A,\F]$, which is now given in terms of both the residual gauge field $A$ and the Higgs scalar $\F$, is that like the CP density it
is also a $total\ divergence$
\[
\Om_{\rm HCP}=\pa_i\Om_i\ ,\quad i=\mu,D\ ;\ \quad\mu=1,2,\dots,d\ ;\ d=D-1\ .
\]

Implementing now the one-step descent of the density $\Om_i$, one can define the corresponding new Chern-Simons density
as the $D$-th component of $\Om_i$, namely $\Om_{\rm HCS}\stackrel{\rm def.}=\Om_D$.
We refer to the quantity $\Om_{\rm HCS}$ as the Higgs--Chern-Simons (HCS) density. A detailed definition of the HCS density is given in
Refs.~\cite{Tchrakian:2010ar,Radu:2011zy,Tchrakian:2015pka}. Subsequently, a similar definition for the HCS density was given
in \cite{Szabo:2014zua},
but only in odd dimensions~\footnote{Apart from the definition in Ref.~\cite{Szabo:2014zua} being restricted to odd dimensions, there is another important difference with with our formulation. In our case the
dimensional reduction is carried out on the {\bf gauge\ invariant} CP density yielding the HCP density, while in \cite{Szabo:2014zua} it is the CS density in the (higher) odd dimensions that is
subjected to dimensional reduction. While the results happen to be similar, there is no guarantee they should agree since subjecting a {\bf gauge\ variant} CS density to symmetry imposition as  done in \cite{Szabo:2014zua} problematic.} and with the Higgs scalar being a complex column, not suited to the application here. In our formulation, HCS densities are given in both odd and even dimensions and in any given dimension,
there is an infinite family of HCP densities in $D$ dimensions, as also HCS densities in $d=D-1$ dimensions, since these follow from the descent of a
CP density in any dimension $N=2n>D$.

Once the Higgs-CS (HCS) densities are calculated, they can be employed to generate gravitational theories in the same spirit
as in \cite{Witten:1988hc,Chamseddine:1989nu,Chamseddine:1990gk}, which could be designated as HCS gravities (HCSG).
In any given dimension, there is an infinite family of such theories, each resulting from the infinite family of HCS densities.

In the passage of the HCS densities to gravitational systems
in $d=D-1$ dimensions, we see from \re{oddd} and \re{higgsevenD2} below, that the gauge group is
chosen to be $SO(d)$ and the Higgs multiplet is chosen to be a
$D$-component $isovector$ of $SO(D)$~\footnote{These choices coincide
with the representations that yield monopoles on $\R^d$ described in\cite{Tchrakian:2010ar} }.
The cornerstone of constructing CSG models is the identification of the non-Abelian (nA) $SO(D)$ connection in $d=D-1$
dimensions~\footnote{We do not make a choice for the signature of the space at this stage.},
with the spin-connection $\om_\mu^{ab}$ and the $Vielbein$ $e_\mu^a$, ($\mu=1,2,3$;\ a=1,2,3). The
prescription employed in \cite{Witten:1988hc,Chamseddine:1989nu,Chamseddine:1990gk} is
\bea
A_{\mu}&=&-\frac12\,\om_{\mu}^{ab}\,\ga_{ab}+\ka\,e_{\mu}^{a}\,\ga_{a4}\quad\Rightarrow\quad
F_{\mu\nu}=-\frac12\left(R_{\mu\nu}^{ab}-\ka^2\,e_{[\mu}^{a}\,e_{\nu]}^{b}\right)\ga_{ab}+\ka\,C_{\mu\nu}^{a}\ga_{a4}\,,\label{oddd}
\eea
$(\ga^{ab},\ga^{a4})$ being the Dirac gamma matrices used in the representation of the algebra of $SO(D)\,,\ D=4$. The constant $\ka$ has
dimensions $L^{-1}$, compensating the difference of the dimensions of the spin-connection and the $Dreibein$. In \re{oddd},
$$R_{\mu\nu}^{ab}=\pa_{[\mu}\om_{\nu]}^{ab}+(\om_{[\mu}\om_{\nu]})^{ab}$$ is the Riemann curvature, and $C_{\mu\nu}^a=D_{[\mu}e_{\nu]}^a$ is the torsion.

Here, in addition to \re{oddd}, we posit the corresponding prescription for the Higgs scalar $\F$,
\bea
2^{-1}\F=(\f^{a}\,\ga_{a5}+\f\,\ga_{45})\  &\Rightarrow& \
2^{-1}D_{\mu}\F=(D_{\mu}\f^{a}-\ka\,e_\mu^a\,\f)\ga_{a5}+(\pa_{\mu}\f+\ka\,e_\mu^a\,\f^a)\ga_{45}
\label{higgsevenD2}
\eea
which clearly displays the $iso$-$four$-$vector$ $(\f^a,\f^4)$, that are split into the $three\ component$ frame-vector
field $\f^a$ and the scalar field $\f=\f^4$. The covariant derivative $D_\mu\F$ of the Higgs scalar features the gravitational covariant
derivative $$D_\mu\f^a=\pa_\mu\f^a+\om_\mu^{ab}\f^b$$ of the frame vector field $\f^a$.
 Indeed, this is a vector field
$\f_\mu=e_\mu^a\f^a$, which however has rather unusual dynamics as will be seen below. It is neither a gauge field nor a
Proca field, rather, it has geometric content.

The fields $(\f^a,\f)$ are not matter fields like, $e.g.$ Maxwell or Yang-Mills, or Skyrme, $etc$. In the latter
cases, the covariant derivatives are not defined by the (gravitational) spin-connection, while here they are as
seen in \re{higgsevenD2}.   In this sense they are like spinor fields.
 An immediate consequence
of this is that theories like the one proposed here can support solutions with torsion.

  Unlike spinors however,  the fields $(\f^a,\f)$ are gravitational coordinates as they originate from the Higgs field
$\F$ of the nA gauge theory, which
itself is a (dimensional) descendent of a (higher dimensional) connection. Thus, as seen from \re{higgsevenD2}, $(\f^a,\f)$
are on the same footing as the $usual$ gravitational coordinates $(\om_\mu^{ab},e_\mu^a)$.
As a consequence, we would expect that the effect of $(\f^a,\f)$ on the solutions cannot be characterised as $hair$. We
expect that they support only  black hole solutions and do not describe horizonless (soliton)
solutions in the limit of the horizon radius vanishing, as it happens in the usual theories with hair.

 The gravitational models resulting from the Higgs-CS (HCS) densities via \re{oddd}-\re{higgsevenD2} are
referred to as HCS gravities~\cite{Tchrakian:2017fdw} (HCSG). In this report we have restricted our detailed study to the
``simplest'' HCSG model in $2+1$ dimensions, namely to the HCSG model resulting from the HCS density descended from
the HCP density in $6$ (rather than those in $8$, $10$, $etc.$) dimensions. This model is an extension of the
$usual$ Chern-Simons gravity~\cite{Witten:1988hc}, and our solutions can be contrasted with the
Banados, Teitelboim and Zanelli
(BTZ)~\cite{Banados:1992wn}
black hole solution in that theory.

This paper is organized as follows.
The model studied is presented in Section {\bf 2}, including the equations of motion. Then in Section {\bf 3} the imposition of (radial)
symmetry is carried out, for the torsion-free case where the spin-connection is restricted to the Levi-Civita connection. There are two
questions that symmetry imposition must address: $a$) The consistency of the Ansatz, and $b$) the consistency of using a torsion-free Ansatz,
in a theory where the torsion tensor cannot be set to zero $a\ priori$ because of the appearance of the gravitational covariant derivative.
Both these questions are addressed implicitly, in Section {\bf 3}. In Section {\bf 4} we present the solutions of the
system  with backreacting HCSG fields.

\section{A HCSG model in $2+1$ dimensions}
The Higgs--Chern-Simons density (HCS) employed here is the ``simplest'' example in $2+1$ dimensions.
By simplest we mean that the Higgs--Chern-Simons (HCS) density employed to construct the HCS gravity (HCSG), is the one resulting from the
``simplest'' Higgs--Chern-Pontryagin (HCP) density, which is defined in one dimension higher, namely in $four$ dimensions. Now in $four$ dimensions,
HCP densities can be constructed as dimensional descendants of a CP density in $2n>4$ dimensions, hence it is reasonable to describe the
``simplest'' case at hand to be the HCP density in $4$ dimensions, the one that descends from the CP density in $2n=6$ dimensions.

Since like the CP density, the HCP density is a $total\ divergence$, then the corresponding HCS density results from usual $one$-$step$ descent,
in this case from $4$ to $3$ dimensions. It may be helpful to display two such HCS densities in $2+1$ dimensions, each resulting from the
$one$-$step$ descent of a HCP density th $4$ dimensions, the first of which has resulted from the dimensional descent of the CP in $6$
dimensions, and the second in $8$ dimensions. These are
\bea
\Omega^{(3,6)}_{\rm HCS}&=&
-2\eta^2\Omega_{\rm CS}^{(3)}-\vep^{\mu\nu\la}\mbox{Tr}\,\ga_5D_{\la}\F\left(F_{\mu\nu}\,\F+F_{\mu\nu} \F\right)\,
,
\label{HCS36}
\\
\Omega^{(3,8)}_{\rm HCS}&=&6\eta^4\Omega_{\rm CS}^{(3)}-\vep^{\mu\nu\la}\,\mbox{Tr}\,\ga_5\,\bigg\{
6\,\eta^2\left(\F\,D_{\la}\F-D_{\la}\F\,\F\right)\,F_{\mu\nu}
\nonumber\\
&&\hspace{20mm}-\bigg[\left(\F^2\,D_{\la}\F\,\F-\F\,D_{\la}\F\,\F^2\right)-2\left(\F^3\,D_{\la}\F-D_{\la}\F\,\F^3\right)\bigg]F_{\mu\nu}
\bigg\}\,,\label{HCS38}
\eea
where the leading term $\Om_{\rm CS}^{(3)}$ in each is the usual CS density
\be
\label{CS3}
\Om_{\rm CS}^{(3)}=\vep^{\mu\nu\la}\mbox{Tr}\,A_{\la}\left(F_{\mu\nu}
-\frac23\,A_{\mu}A_{\nu}\right),
\ee
and where the constant $\eta$ and the Higgs field $\F$ both have the dimensions of $L^{-1}$, like the gauge connection.

Our choice for the ``simplest'' HCS density will be \re{HCS36}, rather than for example \re{HCS38} or ones originating from even higher
dimensional CP densities. Applying the prescriptions \re{oddd} and \re{higgsevenD2}, \re{HCS36} yields the HCS gravitational (HCSG) model
studied here,
\bea
{\cal L}_{\rm HCSG}&=&\vep^{\la\mu\nu}\vep_{abc}\Bigg\{2\eta^2\ka\,\left(e_{\la}^{c}\,R_{\mu\nu}^{ab}
-\frac23\ka^2e_{\mu}^{a}e_{\nu}^{b}e_{\la}^{c}\right)\nonumber\\
&&+\bigg[2(R_{\mu\nu}^{ab}-\ka^2\,e_{[\mu}^{a}e_{\nu]}^{b})\left[\f^{c}(\pa_{\la}\f+\ka\,e_{\la}^d\f^d)
-\f (D_{\la}\f^{c}-\ka\, e_{\la}^c\f)\right]\nonumber\\
&&\qquad\qquad\qquad\qquad\qquad\qquad-4\ka\f^{a}(D_{\la}\f^{b}-\ka\,e_\la^b\f)C_{\mu\nu}^{c}\bigg]\Bigg\},
\label{HCSG2+1}
\eea
where $C_{\mu\nu}^{c}$ is the torsion tensor.

In the Lagrangian \re{HCSG2+1}, both the torsion $C_{\mu\nu}^{c}$ and the covariant derivative $D_{\la}\f^{c}$ are defined
in terms of the spin-connection $\om_\mu^{ab}$, so that the variation w.r.t. to the latter will result in the appearance of the
$C_{\mu\nu}^{c}$ in the field equations. Whether or not can the torsion be set equal to zero
consistently~\footnote{Note that coupling gravity, $e.g.$ to Maxwell, Yang-Mills or Skyrme/Higgs
fields can consistently be considered in a torsionless framework, since the kinetic terms of these fields $do\ not$ feature the spin-connection.}
 for a particular field configuration must be checked. This question is tackled in Section {\bf 3}
where the system is subjected to static radial symmetry.

In the present work, we restrict our attentions to the Levi-Civita connection
\be
\label{L-C}
\om_{\mu}^{ab}[e,\pa e]=-\frac12\,e_{\mu}^d\,e^{\rho a}e^{\si b}\pa_{[\rho}e_{\si] d}+\frac12\,e^{\la [a}\,\pa_{[\mu}e_{\la]}^{b]}\,,
\ee
subject to checking the consistency of our Ansatz with this case.

\subsection{Equations of motion}
To express the equations of motion concisely, it is useful to introduce the notations
\bea
{\cal V}^{\la}_c&=&\vep^{\la\mu\nu}\vep_{cab}(R_{\mu\nu}^{ab}-\ka^2e_{[\mu}^ae_{\nu]}^b)\,,\label{calV}\\
{\cal S}&=&\eta^2-\f^2-|\vec\f|^2\label{calS}\,.
\eea
The (modified) Einstein equations
follow from the variation of \re{HCSG2+1}
$w.r.t.$
 the Dreibein $e_\la^c$, yielding
\bea
\label{Ein}
E_c^\la&=&\ka\,{\cal S}{\cal V}^{\la}_c+4\ka\vep^{\la\mu\nu}\vep_{cab}\left[D_{\mu}\f^aD_{\nu}\f^b
-\ka\f\left(2D_\mu\f^a-\ka\,e_\mu^a\,\f\right)e_\nu^b\right]=0\,.
\eea
The equations
resulting from the variation of the frame-vector scalar $\f^c$ are
\be
\label{fa}
E_c=2{\cal V}^{\la}_c(\pa_\tau\f+\ka\ \vec e_\la\cdot\vec\f)+4\vep^{\la\mu\nu}\vep_{cab}\,C_{\mu\nu}^a\,(D_\la\f^b-\ka\,e_\la^b\f)=0\,,
\ee
while the equation
resulting from the variation of the scalar $\f$ is
\be
\label{eqf}
E=-2{\cal V}^{\la}_c\,(D_\tau\f^c-\ka\,e_\la^c\f)=0\,.
\ee
The torsion equations
follow from the variation of \re{HCSG2+1} w.r.t. the spin connection $\om_\la^{ab}$,
not constrained to be the Levi-Civita connection \re{L-C}, yielding
\bea
E_{ab}^\la&=&\vep^{\la\mu\nu}\vep_{cab}\Bigg\{-2\ka\,{\cal S}C_{\mu\nu}^c+8D_\mu\f^c\,\pa_\nu\f+\nonumber\\
&&\qquad\qquad+8\ka\left[(\vec e_\nu\cdot \vec\f)D_\mu\f^c+e_\nu^a\,\f\pa_\mu\f\right]-8\ka^2\f(\vec\f\cdot\vec e_\nu)e_\mu^c\Bigg\}=0
\label{torseq}
\eea
Note that in \re{torseq} the curvature $R_{\mu\nu}^{ab}$ does not appear. Setting $C_{\mu\nu}^a=0$
in \re{torseq} puts a constraint on the fields $(\f^a,\f)$,
which for consistency should be satisfied for a given field configuration.

In \re{Ein}, in \re{torseq} and in \re{fa}, the ``usual'' notation $|\vec\f|^2=\f^a\f^a$, $(\vec e_\tau\cdot\vec\f)
=e_\mu^a\f^a$ and $(\vec e_\mu\cdot D_\nu\vec\f)=e_\mu^aD_{\nu}\f^a$ is used.

Also, in what follows we opt for Minkowskian signature and make the replacement
\be
\label{replace}
\ka\to i\ka\ ,\quad h\to -ih\,.
\ee
As such, setting $\phi=\phi^a=0$
results in Einstein gravity with a negative cosmological constant
$\Lambda=-\kappa^2$.
As found in \cite{Banados:1992wn}
by  Banados, Teitelboim and Zanelli
(BTZ),
this model possess black hole (BH) solutions with
Anti-de Sitter asymptotics.
Their study has been seminal for a better understanding of
BH physics and dualities.

A natural question, which we propose to address in the
following Section,
is if the BTZ BHs possess generalizations
within the full model
(\ref{HCSG2+1})
with excited functions $\phi,\phi^a$.

\section{The solutions}

\subsection{The Ansatz}

We convert the usual static radially symmetric metric Ansatz in $2+1$ dimensions
\bea
\label{metric}
ds^2=A^2(r)dr^2+r^2d\vf^2-B^2(r)dt^2,
\eea
(where
$r,t$ are the radial and time coordinate, respectively,
while $0\leq \varphi <2\pi$),
to the corresponding Dreibein Ansatz as follows
\bea
\label{DreiAnsatz}
&&e_{r}^{\al}=A\,n_{(1)}^{\al}\ ,\qquad e_{\vf}^{\al}=r\,n_{(2)}^{\al}\ ,\qquad e_{t}^{3}=B,
\label{e+}
\eea
where
\be
\label{n}
n_{(1)}^{\al}=\left(\begin{array}{l}
\cos n\vf\\
\sin n\vf
\end{array}
\right)=(\vep n_{(2)})^\al\ ,\quad
n_{(2)}^{\al}=\left(\begin{array}{l}
-\sin n\vf\\
\ \ \cos n\vf
\end{array}
\right)=-(\vep n_{(1)})^\al,
\ee
where $n$ is an integer.

The Ansatz we use for the frame-vector field $\f^a=(\f^{\al},\f^3)$ and the scalar $\f$ is
\bea
\f^{\al}&=&f(r)\,n_{(1)}^{\al}\ ,\quad\f^3=g(r)\label{fal3},
\\
\f&=&h(r)\,,
\label{f}
\eea
having used the same unit vector $n^{\al}_{(1)}$ in \re{fal3} as that given by \re{n}.

We restrict our attention to the torsion-free case, substituting the Ansatz \re{e+}
in the Levi-Civita connection
\re{L-C} and calculating the resulting components of the curvature. Using this reduced spin connection and the Ansatz
\re{fal3}-\re{f}, we calculate the reduced (covariant) derivatives of the fields $(\f^a,\f)$.
Substituting all this in the
equations \re{Ein}, \re{fa} and \re{eqf}, we find that these are satisfied for $g(r)=0$.
Thus there remain
four equations for the functions $(A,B,f,h)$, plus one constraint equation that is satisfied.
We then substitute this torsion-free Ansatz in the torsion equations \re{torseq}, yielding three non-trivial equations,
each of which is satisfied by the ``Einstein'' equation for $h'$.
Therefore
we conclude that our torsion-free Ansatz is consistent.

We also remark that the system is described by the
reduced Lagrangian resulting from the imposition of symmetry on \re{HCSG2+1},
\bea
\label{redlag}
4^{-1}L_{\rm HCSG}&=&2\eta^2\ka\left[-\frac{BA'}{A^2}+\ka^2rAB\right]\nonumber\\
&&-\bigg\{2\left(\frac{B'}{A^2}\right)fh'+\frac{\ka}{A}\left[\left(\frac{BA'}{A}\right)(g^2-h^2)-B'(f^2+2rhh')\right]\nonumber\\
&&\qquad+\ka^2\left[(rB'+B)fh-rB(fh'-hf')\right]+\ka^3rAB(f^2+g^2-3h^2)\bigg\}\,.
\eea
We observe that, indeed, \re{redlag} does not feature the derivative of the function $g(r)$, and hence one can
consistently set $g(r)=0$.

   \subsection{An exact solution (HBTZ BH
   }
  In the absence of the fields $(\f^a,\f)$, only the equation \re{Ein} must be solved, which is of course satisfied
by the vacuum BTZ solution~\cite{Banados:1992wn}. Since the BTZ solution satisfies the equations of
Chern-Simons gravity
(CSG) in $2+1$ dimensions, and since the solution presented here results instead from the equations of the Higgs--Chern-Simons
gravity (HCSG), one might refer to the new solutions as Higgs-BTZ, or simply as HBTZ black holes.

We have found that the field equations  (\ref{Ein})-(\ref{eqf}) possess a closed-form solution with
\bea
B^2(r)&=&\frac{1}{A^2(r)}=\ka^2  r^2+c_t,
\label{solnsAB}
\\
h(r)&=&c_0r\ ,\quad f(r)=\frac{c_0}{\ka}B(r),
\label{solnshf}
\eea
where $c_t, c_0$ are free parameters. Equivalently, \re{solnshf} can be replaced by $(f,h)\to(h,f).$

One can see that (\ref{solnsAB})
corresponds to a globally AdS$_3$
geometry (for $c_t>0$) or to a BTZ black hole (for $c_t<0)$,
which are solutions of  the Einstein equations also for $\phi^a=\phi=0$.
Thus the fields $(\phi^a,\phi)$
do not backreact on these geometries, leading to
a vanishing {\it effective} energy-momentum tensor, $i.e.$ that these solutions are {\it effectively} vacuum solutions~\footnote{
   It is interesting to note the analogy with  gravitating  self-dual instantonic Yang-Mills configurations
   with Euclidean metric
see e.g. \cite{Charap:1977ww}, \cite{Brihaye:2006bk}, \cite{Radu:2007az}.  In that case the reason is that the stress tensor vanishes identically due to self-dualty. In the present case, (\ref{solnsAB}),  (\ref{solnshf})
are solutions also for an Euclidean signature
and one can easily check that the contribution of the
second term in (\ref{HCSG2+1})
to the total action is nonvanishing.
Based on this analogy, one might claim that these closed form solutions are {\it effectively} vacuum solutions.
}.
This solution possesses another unusual property, namely that $f$ and $h$ functions diverge at infinity.

One may ask if other solutions exist
apart from  (\ref{solnsAB}),  (\ref{solnshf})
(preferably with both $f$ and $g$
finite in the far field).
The answer seems to be negative,
a strong indication
in this direction coming from the study of the near horizon expansion of the solutions.
The first step here is to notice that the
field equations imply that the function $f$ can be eliminated, with
 \begin{eqnarray}
f(r)=\frac{h'(r)}{\kappa A(r)},
\end{eqnarray}
The BH solutions
possess an  horizon at $r=r_H>0$,
where we suppose  the following approximate form of the
generic solution
(with
$A(r)=\frac{1}{\sqrt{U(r)}},~B(r)=\sqrt{H(r)}$):
   \begin{eqnarray}
     \label{pert}
H(r)=\sum_{k\geq 0}H_{(k)}(r-r_H)^k,~~
U(r)=\sum_{k\geq 0}U_{(k)}(r-r_H)^k,~~
h(r)=\sum_{k\geq 0}h_{(k)}(r-r_H)^k,~~
\end{eqnarray}
where $H_{(k)}$, $U_{(k)}$ and $h_{(k)}$ are real numbers.
After substituting  \re{pert} in the equations of motion and solving order by order, we have found
that
\begin{eqnarray}
&&
H(r)= H_{(1)}(r-r_H)+\frac{H_{(1)}}{2r_h}(r-r_H)^2+O(r-r_H)^{12},
\\
&&
U(r)= 2\kappa^2 r_H(r-r_H)+\kappa^2 (r-r_H)^2+ O(r-r_H)^{12},
\\
&&
h(r)=\frac{h_{(0)}}{r_H}r+O(r-r_H)^{11}.
\end{eqnarray}
The above result has been proven up to order $11$ in
perturbation theory. It is likely however, that it holds to all orders, although we do not have a proof of that.
This coincides with the near horizon form of the exact solution
(\ref{solnsAB}),
(\ref{solnshf})
(note that the metric function $B(r)$ is fixed up to a constant factor
$B(r)\to \lambda B(r)$ ).
Thus we conclude that
(\ref{solnsAB}),
(\ref{solnshf})
is
likely
 the unique configuration compatible with a regular expansion at the horizon\footnote{This also
agrees with our numerical results, which
have failed to indicate the existence of other solutions apart from
(\ref{solnsAB}),
(\ref{solnshf}).}.

A similar argument excludes the existence of particle-like solitonic solutions
apart from
(\ref{solnshf})
in an  AdS background.

\subsection{Deformed charged HBTZ black holes}

The above results,  namely the HBTZ solution, are
consistent with the spirit of the 'no hair' theorems, which
exclude the existence of BH solutions with matter fields that do not possess
measured quantities subject to  a Gauss Law
\cite{Bekenstein:1996pn},
\cite{Volkov:1998cc},
\cite{Herdeiro:2015waa}.

The 'no hair' constraints can be circumvented for
more complicated models,
typically possessing gauge fields
(see $e.g.$
\cite{Gubser:2008px},
\cite{Gubser:2008zu},
\cite{Winstanley:1998sn},
	for seminal work on hairy black holes with AdS asymptotics).
Thus one can ask if the results in the previous subsection are generic and hold also in more general models,
with a Lagrangian containing matter
fields in addition to fields  $(e_\mu^a,\phi^a,\phi)$.

To address this question, we consider the simplest generalization of the model
(\ref{HCS38}),
with an additional Maxwell term,
\begin{eqnarray}
\label{new-model}
{\cal L} = {\cal L}_{\rm HCSG}-\frac{1}{4}F_{\mu\nu}^2,
\end{eqnarray}
with $F_{\mu\nu}=\pa_{[\mu}A_{\nu]}$ the field strength tensor. It is clear that in this case there will be a
nonvanishing stress tensor.

Considering the same {\bf metric} Ansatz (\ref{metric}),
we take a purely electric connection
\begin{eqnarray}
A_\mu=(A_0,A_i)=(V(r), 0)~.
\end{eqnarray}
The corresponding equations are easily derived;
note that
$V(r)$ interacts with $(\phi^a, \phi)$ only via the geometry, with the existence of a first integral
\begin{eqnarray}
     \label{firstint}
V=\int dr \frac{Q}{r}\sqrt{AB},
\end{eqnarray}
where $Q$ is an integration constant
identified with the electric charge.

For $f=g=h=0$,
the  electrically  charged BTZ BH \cite{Banados:1992wn} is recovered, with
\be
\label{charged-BTZ}
B^2(r)=\frac{1}{A^2(r)}=\ka^2r^2-M-\frac{Q^2}{2\kappa}\log r~.
\ee
This solution possess an event horizon at $r=r_H$, where
$B(r_H)=0$.

We are interested in generalizations of this solution with nonvanishing fields $(f,h)$.
Assuming the existence of a regular event horizon at $r=r_H>0$, the field equations
imply the following approximate form of the solutions near the horizon,
\begin{eqnarray}
\label{eh1}
&&
\frac{1}{A^2(r)}=H_1 \kappa^2 r_H^2 (r-r_H)+\dots,~~
B^2(r)=\kappa^2 r_H^2 u_1(r-r_H)+\dots,~~
\\
\nonumber
&&
f^2(r)=h_1^2 H_1r_H^2(r-r_H)+\dots,~~
h(r)=h_0+h_1(r-r_H)+\dots,~~
\end{eqnarray}
in terms of two free parameters $(h_0,u_1)$, with
\begin{eqnarray}
\label{eh2}
&&
H_1=\frac{2}{r_H}
\left(
1+\frac{Q^2}{6(2+h_0^2)\kappa^3 r_H^2}
 (
\sqrt{1-\frac{12h_0^2\kappa^3 r_H^2}{Q^2}}-1
 )
\right),
\\
&&
\nonumber
h_1=\frac{1}{2h_0H_1r_H^2}
\left(
(2+3h_0^2)(2-H_1r_H)+2h_0^2H_1r_H
-\frac{Q^2}{\kappa^3r_H^2}
\right)~.
\end{eqnarray}
Note that the condition for $H_1$ to be real
implies the existence of a maximal value of the functions $h(r)$
at the horizon
\begin{eqnarray}
\label{cond}
h(r_H)<\frac{Q}{2\kappa r_H \sqrt{3\kappa}}\,.
\end{eqnarray}

 \begin{figure}[h!]
\begin{center}
\includegraphics[width=0.55\textwidth]{generic.eps}
\caption{ The parameter $c_0$
which enters the far field asymptotics of the functions $f(r),h(r)$
(with  $(h(r),f(r)) \to c_0 r$),
is shown as a function of the value of $h(r)$ at the horizon,
for as set of generic solutions.
The inset shows a typical profile of the functions $f(r),h(r)$.
}
\label{datagen}
\end{center}
\end{figure}

  We seek electrically charged HBTZ solutions deforming the charged BTZ BH's, with the functions $(f,h)$ excited. We have encountered solutions that possess isolated zeros of $(f,h)$ for some values of $r$, $i.e.$, displaying nodes, whose detailed study we have eschwewd. Henceforth we concentrate exclusively on {\it nodeless, fundamental} solutions.

Generic solutions with non-standard asymptotics are found for the near horizon expansion (\ref{eh1}).
As seen in Figure \ref{datagen},
similar to the exact solution
(\ref{solnshf}),
the fields $(f,h)$ diverge linearly as $r\to \infty$,
with  $(h(r),f(r)) \to c_0 r$.
This divergence mixes with the logarithmic terms originating in the Maxwell
part of the theory, leading to a slower decay at infinity of the functions $B^2/r^2$ and $A^2r^2$, as compared to the charged BTZ case.

 In addition to these generic solutions, we have found special solutions isolated in parameter space.
For given (and nonzero) $(r_H,Q)$, a different situation is found for a particular set of
near-horizon parameters $(h_0,u_1)$, which lead to $f$ and $h$ vanishing at infinity, with $c_0=0$
(for the data exhibited in Figure \ref{datagen}, this corresponds to the blue point).

The resulting configurations possess the following large-$r$ asymptotic expansion:
\begin{eqnarray}
\label{inf1}
&&
 A^2(r)=\frac{1}{\kappa^2 r^2}+
\left(
\frac{c_t-4  c_s^2}{\kappa^2}+\frac{ Q^2}{2\kappa^5}\log r
\right)
\frac{1}{r^4}
+\dots,
~~
B^2(r)=
\kappa^2 r^2-c_t  -\frac{  Q^2}{2\kappa^5}\log r+\dots,
\\
&&
f(r)=-\frac{c_s}{r}+\dots,~\qquad\qquad\qquad\qquad\qquad\qquad\qquad h(r)=\frac{c_s}{r}+\dots,~
\end{eqnarray}
in terms of two constants
$c_t$,
$c_s$.

This set of  solutions are of particular interest and, for the remainder of
this Section we shall {\bf confine our} discuss{\bf ions to} their basic properties.
These BHs are constructed numerically by using a standard ordinary differential equation solver.
In our approach, we evaluate
the initial conditions
(\ref{eh1})
at $r = 10^{-5}$ for global tolerance $10^{-14}$,
adjusting for fixed shooting
parameter and integrate the equations towards $r\to \infty$
where the far field asymptotics (\ref{inf1}) are approached.
The profiles of a typical solution is displayed in Figure 1.

 \begin{figure}[h!]
\begin{center}
\includegraphics[width=0.55\textwidth]{profile.eps}
\caption{ The profile of a typical black hole solution with nontrivial
$(\phi^a,\phi)$-fields.
}
\label{profile}
\end{center}
\end{figure}

 \begin{figure}[h!]
\begin{center}
\includegraphics[width=0.55\textwidth]{data.eps}
\caption{ Relevant data is shown for a family of charged black hole solutions.
}
\label{data}
\end{center}
\end{figure}

   The resulting solutions can be interpreted as deformations of the charged BTZ BHs,
 since the fields $(\phi^a,\phi)$ in this case deform the geometry
on and outside the horizon.
 To highlight the departure of the charged (deformed) HBTZ BH from the charged BTZ BH, we consider some relevant thermodynamic quantities.
Their Hawking temperature $T_H$ and
event
 horizon area
$A_H$
 are unambiguously defined,
with
\begin{eqnarray}
\label{TH}
T_H=\frac{\kappa^2 r_H^2}{4\pi}\sqrt{H_1 u_1},~~A_H=2\pi r_H.
\end{eqnarray}
For $f=h=0$, the mass of the solutions is determined by the constant $c_t$
in the far field asymptotics (\ref{inf1}),
while the entropy is $S=A_H/4$.
However,
given the direct coupling of the
 coupling of matter fields $\phi^a,\phi$ with the curvature tensor,
 the definition of the BH mass and entropy for the general model (\ref{new-model})
is not $a\ priori$ clear, this issue requiring a separate study.

A number of basic properties of the  solutions are shown in Figure 3.
One can see that, similar to the charged BTZ case, there is a single branch of solutions,
with both $c_t$ and $T_H$ increasing with $A_H$.
Moreover, for the same horizon size, the solutions with nonzero $(f,h)$ are warmer.
Interestingly, the solutions possess a zero temperature extremal limit,
which is nonsingular and featurs a nonvanishing horizon size.
The deviation\footnote{The solutions possess a second parameter, $c_s$, in
the far field expansion (\ref{inf1}),
which can be interpreted as a scalar 'charge',
and provides annother measure for
the deviation of  charged HBTZ BH from the (usual) charged BTZ BH.
Note however, that no global charge is a associated with $c_s$.
} from the standard charged BTZ BH is maximal, close
to that limit,  while the fields $(\phi^a,\phi)$
trivialize for large horizon size,
$(f,g)\to 0$ as $r_H\to \infty$.

\section{Summary and outlook}

   In this paper we have studied a generalization of the familiar Chern-Simons gravity (CSG) in $2+1$ dimensions proposed in
   Ref.~\cite{Witten:1988hc}, where
   the gravitational model is described by both the Einstein-Hilbert (EH) Lagrangian with a (negative) cosmological constant. In our
   generalized model, in addition to the EH and cosmological terms, our Lagrangian features new terms described by a frame-vector
   field $\f^a$ and a scalar field $\f$. The dynamical terms of the fields $(\f^a,\f)$ are non-standard~\footnote{By standard, we mean
   that the dynamical term of the field $\f_\mu=e^a_\mu\f_a$ would feature the {\it square} of the velocity field $\pa_\mu\f_\nu$.}.

   The generalization that introduces the fields $(\f^a,\f)$ is a result of the following.
	While the construction of Chern-Simons gravities
   in all odd dimensions employs~\cite{Witten:1988hc}\cite{Chamseddine:1989nu,Chamseddine:1990gk} non-Abelian Chern-Simons densities, we
   employ instead an alternative type of generaized CS densities that we have referred to as
   Higgs--Chern-Simons~\cite{Tchrakian:2010ar,Radu:2011zy,Tchrakian:2015pka} (HCS) densities. The HCS densities are extracted from the
   Higgs--Chern-Pontryagin~\cite{Tchrakian:2010ar} (HCP) densities, which being descendents of Chern-Pontryagin (CP) constitute an infinite
   family in any $even$ given, including {\it even} spacetime dimensions.
This construction is described in Ref.~\cite{Tchrakian:2017fdw}.
The present work is a first exploration of such gravitational models, and we have chosen the lowest
   dimension, $2+1$, and simplest model in this dimension, which employs the HCS density extracted from the $3$-rd
   CP density in $6$ dimensions.

   The HCS gravity model we have studied, \re{HCSG2+1}, features the gravitational covariant derivatives of the frame vector field $\f^a$,
   $a=1,,2,3$ in this case, so that the possibility of finding non-zero torsion solutions is not excluded. Here we have chosen to seek only
   torsion-free solutions. We have constructed radially symmetric solutions employing the usual metric~\cite{Banados:1992wn} Ansatz,
   augmented by a suitable Ansatz for the fields $(\f^a,\f)$. We have verified the consistency of our Ansatz, and what is more is, that we
   have verified that the torsion equations resulting from the variation of \re{HCSG2+1} with respect to the spin-connection are identically
   satisfied by the equations resulting from the variation of \re{HCSG2+1} with respect to the metric fields, in {\it this} Ansatz.

   We have found a closed form solution analogous to the BTZ~\cite{Banados:1992wn} black hole, which we have referred to as a
   Higgs-BTZ HBTZ black hole (BH). We have a heuristic verification of the fact that this HBTZ BH is unique, and most importantly that
   there are no regular solutions in this model. In this respect, the HBTZ BHs cannot be considered as hairy solutions,
   as would have been the case if matter fields were present and the solutions persisted in the limit of vanishing
   horizon radius. As such, the fields $(\f^a,\f)$ should not be seen as matter fields.

   With the intention of introducing a matter field, we have extended our model to feature a Maxwell term.
   We have sought, and found, new solutions by adding the Maxwell field to \re{HCSG2+1}. As in the case of the electrically charged BTZ
   BH~\cite{Banados:1992wn}, the Abelian matter does not result in hairy solutions and the solutions we find are qualitatively similar to the
   electrically charged BTZ BH. Unlike the latter however, these electrically charged HBTZ BHs are not given in closed form but are
   constructed numerically. We have found it useful to consider some thermodynamic properties of the electrically charged HBTZ BHs, by way
   of contrasting them to the electrically charged BTZ BHs.

   As this is a preliminary exploration of such systems, there is a long list of follow-up investigations, which we list:

   \begin{itemize}
   \item
     Seek torsionful solutions in the model studied here.
   \item
     Analyze the present model, augmented by the planar Skyrme model in $2+1$ dimensions, by way of introducing a metter field.
     This would be an alternative to the Maxwell field considered here as a matter field. We expect that with the Skyrme matter,
     regular solutions in the limit of vanishing horizon radius may exist.
   \item
     Consider the HBTZ BHs in $2+1$ dimensions, of the next HCSG model in the hierarchy, namely \re{HCS38} that results from
     the dimensional reduction of the $4$-th CP density in $8$ dimensions. We expect the resulting HBTZ BH to be qualitaively similar
     to the one studied here.
   \item
     Consider the HBTZ BHs in $4+1$ and $6+1$ dimensions, in the HCSG models constructed from HCS densities extracted from HCP densities
     descended from the $4$-th and $5$-th CP densities given in Ref.~\cite{Tchrakian:2017fdw}.

     This would throw light on some general properties of HCSG BHs in all odd dimensions, analogous to the property common to CSG BHs
     in all odd dimensions, namely that the simplest solutions posesses a generic form with $\frac{1}{g_{rr}}=-g_{tt}=\ka^2r^2+c_t$,
     starting with the BTZ BH in $2+1$ dimensions.
   \item
     Consider the HBTZ BHs in $3+1$ dimensions, in the HCSG models constructed from HCS densities extracted from HCP densities
     descended from the $3$-rd and $4$-th CP densities~~\cite{Tchrakian:2017fdw}. This would be a novel result in that Chern-Simons
     gravitational BHs in {\it even} dimensional spacetimes may also be of some interest.
   \end{itemize}

   In addition to the above systematic follow-ups, it is possible to consider a more formal possibility. This is the analogue of augmenting
   a given gravitational Lagrangian, with a gravitational Chern-Simons (GCS) term, most familiary known since a long time from
   Ref.~\cite{Deser:1982vy} where the usual Einstein Lagrangian was augmented by the GCS term in $2+1$ dimensions. In the present case
   for example, one might consider the gravitational Higgs--Chern-Simons term (GHCS), since this one features the same field multiplets.
   $(e_\mu^a,\f^a,\f)$ as the HCSG model studied. (The definitions of GCHS terms, along with the usual GCS densities, is given in
   Ref.~\cite{Tchrakian:2017fdw}. These are derived from a {\it modified version}~\footnote{In odd dimensions, where the HCS term is
   extracted from a HCP term in even dimensions, the chiral matrix under the Trace of ther latter must be removed {\it by hand}. This
   {\it ad hoc} step is taken so that the leading term in the GHCS density is the GCS density in the given dimension. This question does not
   arise in even dimensional spacetimes.
   .} of the HCS densities rather than from the CS densities in the $usual$ case.)

The simplest such GHCS term in $2+1$ dimensions, which has the same dimensions as \re{HCSG2+1}, is
\bea
\hat\Om_{\rm GHCS}^{(3,6)}&=&-2\eta^2\hat\Om_{\rm GCS}^{{(3)}}+4\vep^{\la\mu\nu}\,\f^a R_{\mu\nu}^{ab}D_\la\f^b,
\label{GHCS36}
\\
\hat\Om_{\rm GCS}^{{(3)}}&=&-\frac{1}{2}\,\vep^{\la\mu\nu}
\om_{\la}^{ab}\left[R_{\mu\nu}^{ab}-\frac23\left(\om_{\mu}\om_{\nu}\right)^{ab}\right],
\label{GCS31}
\eea
$\hat\Om_{\rm GCS}^{{(3)}}$ in \re{GCS31} being the usual GCS term used in Ref.~\cite{Deser:1982vy,Deser:1981wh}.
Note that the GHCS density \re{GHCS36} features only the frame-vector field $\f^a$ and not the scalar $\f=\f^4$, while the latter
is present in the HCSG model \re{HCSG2+1}.

Perhaps more interesting are the first two GHCS densities in $3+1$ dimensions, each derived from the HCS
densities extracted, respectively, from HCP density densities in $6$ and in $8$ dimensions. These are
\bea
\hat\Om_{\rm GHCS}^{(4,6)}&=&
-\frac14\,\vep^{\mu\nu\rho\si}\,R_{\mu\nu}^{ab}\,R_{\rho\si}^{ab}\,\f\label{GHCS46}\\
\hat\Om_{\rm GHCS}^{(4,8)}&=&
-\vep^{\mu\nu\rho\si}\,
R_{\mu\nu}^{ab}\left\{\left[\frac18\left(1-\frac{1}{3}(|\f^a|^2+\f^2)\right)R_{\rho\si}^{ab}
+\frac13\,\f_{\rho\si}^{ab}\right]\f+\frac43\f^{a}D_{\rho}\f^{b}\,\pa_{\si}\f\right\}\label{GHCS48}
\eea
where the abbreviated notation
\[
\f_{\mu\nu}^{ab}=D_{[\mu}\f^a D_{\nu]}\f^b\ , \quad a=1,2,3,4\ ;\quad{\rm and}\quad \f=\f^5\,.
\]
                              The reason for displaying \re{GHCS48} in addition to \re{GHCS46} is that the former does not feature any
                              dynamical terms for $(\f^a,\f)$, while the latter does. The GHCS densities \re{GHCS46} and \re{GHCS48}
                              can be viewed as alternatives to the GHCS density proposed in Ref.~\cite{Jackiw:2003pm}.

 \medskip
\noindent {\large\bf Acknowledgements}
\\
We are grateful to Ruben Manvelyan for helpful discussions throughout this work, and to Hermann Nicolai for hospitality at the
Albert-Einstein Institute for Gravitational physics (Golm), where this work was started.
Thanks to
Brian Dolan,
Carlos Herdeiro,
Olaf Lechtenfeld
and Shahin Sheikh-Jabbari for helpful comments.
E.R. acknowledges funding from the FCT-IF programme and is
also partially supported by the  H2020-MSCA-RISE-2015 Grant No.  StronGrHEP-690904,
the H2020-MSCA-RISE-2017 Grant No. FunFiCO-777740,
and by the CIDMA project UID/MAT/04106/2013.

\begin{small}

redpajama_set_name: RedPajamaArXiv


text:
Book Reviews, Novels
Ronald Sukenick's UP (1968)
Ronald Sukenick was one of the founders and vocal leaders of the Fiction Collective back in '68, a club of (largely) New York innovators taking advantage of the postmodern, self-reflective revolution they were simultaneously witnessing and instigating in literature. They — including authors like Steve Katz and Jonathan Baumbach — argued for an embracing of verbal tricks, of cut-and-paste visual collages in place of story progression, accompanied by a self-awareness of their own limits and possible stylistic pretensions in order to combat the novel's stagnation. Does it add to literature? Does such a question matter, when the novel itself is the author unloading his soul and dumping all his relationship issues out on the reader in as humorous and creative a way he can cough up, no boundaries considered?
A revolutionary of the literary form, he sits today known only among the postmodern literati and English professors. Most of his work is currently out of print.
UP is a legendary novel both good and bad; in some ways it's nothing more than a slow-jerk of self-satisfied, self-obsessed snark, as well as a misogynistic representation of the male-dominated New York publishing industry: Like so many of his FC/early post-modernist peers, women are nothing more than sexual jokes and attractions for the male reader, only reaching that faint trace of genuine humanity when tugging at the author's past regrets and failures. (While I wouldn't have minded this a few years ago, it only upsets me now and hurts my impression of the book.)
Sukenick in the early '70s, around the creation of the Fiction Collective.
UP lacks a trace of linearity, or even a border between fantasy and reality; flowing back and forth, sometimes mid-paragraph, between times, fantasies, sexual misadventures both real and imagined, perspectives, focuses, etc. Sukenick, the writer, is the only constant. Sometimes a failing professor of English pushing himself towards employment; other times a slumming New Yorker writing his own novel as the pages go by, rats infesting the framework; then and before a teenage dreamer reaching for a degree in God-knows-what; simultaneously his alter-ego: A hyper-misogynist Mary Sue interacting with the real Sukenick; oftentimes a sack of lost chances dealing in broken dreams with a partially fictionalized love interest. The real author discusses his upcoming novel with associates, asking them what they think of the parts yet to happen: He's given anything but praise.
Sukenick ends his book with a literal literary classroom revolution, a segue to a party celebrating his book, a book he seems to know is a weak imitation with nothing to say however hard he tries to innovate and say something. All the novel's characters, lost romances, and even his defeated alter-ego, Strop Banally, appear to disregard his work.
The trip's a lot of fun while it lasts, but its of-its-time '60s romantic qualities make the forever-underground status understandable. Unless you're this book's core audience, unless you're a frustrated English academic or a fan of the self-aware post-modernist movement this book helped launch, there's no reason to ever get UP: Either stay away or continue the dig.
"Our generation is a sacrifice to history. When a creative writing student asks me what to write about I answer: Amuse yourself. There's nothing to write about….I see what you're going for. Writing as self-expression and all that. The Romantic gambit. But you can't go back. Between crisis and catastrophe who cares about your ego? Your complaint, your indignation, your outrage—your boils, your hangnails, your stomach aches. It turns to self-pity. This just bores us, we have the same problems. You ought to stick to comedy….Now don't go and blame yourself. This is just the trouble. You're helpless. It's history. It's politics. It's capitalism. It's the literary situation. We're all paralyzed."
Tagged Larry McCaffery's Top 100, Literary Fiction, Misogyny, PoMo, Review, Ronald Sukenick
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text:
Der Wettkampf im Hammerwurf der Männer bei den Olympischen Spielen 2020 in Tokio fand am 2. August 2021 (Qualifikation) und 4. August 2021 (Finale) im neuerbauten Nationalstadion statt.

Olympiasieger wurde der Pole Wojciech Nowicki. Der Norweger Eivind Henriksen gewann die Silbermedaille. Bronze ging an den Polen Paweł Fajdek.

Aktuelle Titelträger

Rekorde

Bestehende Rekorde

Der nun schon seit 33 Jahren bestehende olympische Rekord wurde auch bei diesen Spielen nicht erreicht. Der weiteste Wurf gelang dem polnischen Olympiasieger Wojciech Nowicki mit seinem dritten Versuch im Finale am 4. August auf 82,52 m. Damit blieb er 2,28 m unter dem Olympia- und 4,22 m unter dem Weltrekord.

Rekordverbesserungen
Ein Landesrekord wurde viermal verbessert:
 78,79 m – Eivind Henriksen (Norwegen), erster Versuch in der Qualifikation (Gruppe B) am 2. August
 79,18 m – Eivind Henriksen (Norwegen), erster Versuch im Finale am 4. August
 80,31 m – Eivind Henriksen (Norwegen), dritter Versuch im Finale am 4. August
 81,58 m – Eivind Henriksen (Norwegen), fünfter Versuch im Finale am 4. August

Legende
Kurze Übersicht zur Bedeutung der Symbolik – so üblicherweise auch in sonstigen Veröffentlichungen verwendet:

Qualifikation
Die Athleten traten zu einer Qualifikationsrunde in zwei Gruppen an. Fünf Wettbewerber (hellblau unterlegt) übertrafen die den direkten Finaleinzug Weite von 77,50 m. Damit war die Mindestanzahl von zwölf Finalteilnehmern nicht erreicht. So wurde das Finalfeld mit sieben weiteren Wettbewerbern (hellgrün unterlegt) aus beiden Gruppen nach den nächstbesten Weiten aufgefüllt. Für die Teilnahme am Finale waren schließlich 75,73 m zu erbringen.

Gruppe A

2. August 2021, 9:00 Uhr (2:00 Uhr MESZ)

Gruppe B

2. August 2021, 10:30 Uhr (3:30 Uhr MESZ)

Finale

4. August 2021, 20:15 Uhr (13:15 Uhr MESZ)

Der Hammerwurfwettbewerb war wie eine ganze Reihe weiterer Konkurrenzen bei diesen Spielen von ausgesprochen hoher Qualität. Dass der seit 33 Jahren bestehende olympische Rekord nicht fiel, ist dabei nicht wirklich besonders verwunderlich, auch andere Rekorde gerade in den technischen Disziplinen haben sicherlich auch aufgrund einer im Laufe der Jahre veränderten Dopingkontrollpraxis eine sehr lange Bestandsdauer.

Favorisiert waren in erster Linie die beiden Teilnehmer aus Polen. Pawel Fajdek trat als unter anderem vierfacher Weltmeister (2013/2015/2017/2019) und Europameister von 2016 an. Wojciech Nowicki war der amtierende Europameister und hatte Bronze gewonnen bei den Spielen 2016, den Europameisterschaften 2016 sowie den Weltmeisterschaften 2015, 2017 und 2019.

Nowicki setzte sich mit dem einzigen Wurf jenseits von achtzig Metern (81,18 m) in der ersten Versuchsreihe gleich an die Spitze und steigerte sich mit seinem zweiten Wurf auf 81,72 m. In Durchgang zwei übertraf auch der Ukrainer Mychajlo Kochan die 80-Meter-Marke und lag mit 80,39 m auf dem zweiten Platz. Mit seinem dritten Versuch knackte der Norweger Eivind Henriksen ebenfalls die 80-Meter-Marke – es war sein zweiter norwegischer Rekord im Finale, nachdem er bereits in der Qualifikation einen Landesrekord aufgestellt hatte. Mit 80,31 m war er nun Dritter. Nowicki verbesserte sich derweil weiter auf jetzt 82,52 m.

In der Finalrunde der besten Acht passierte anfangs nicht viel, außer Nowicki kam niemand auf eine Weite jenseits von achtzig Metern. Aber der fünfte Durchgang hatte es noch einmal in sich. Eivind stellte mit nun 81,58 m einen weiteren nationalen Rekord auf und lag damit auf Platz zwei. Fajdek zog mit 81,53 m an Kochan vorbei auf den Bronzerang. Nowicki zeigte mit 82,06 m noch einmal seine Überlegenheit in diesem Wettbewerb. In Runde sechs änderte sich nichts mehr an der Rangfolge, der sechstplatzierte Brite Nick Miller steigerte zwar noch einmal seine Weite, nicht aber seine Platzierung.

So gab es einen souveränen Sieg für Wojciech Nowicki, der mit allen seinen fünf gültigen Versuchen weiter als 81 Meter warf. Überraschender Silbermedaillengewinner wurde Eivind Henriksen. Pawel Fajdek brachte sich mit seiner starken Weite aus dem fünften Durchgang auf den Bronzerang. Auch der viertplatzierte Mychajlo Kochan hatte in seinem Endresultat noch eine Weite von mehr als achtzig Metern aufzuweisen. Auf den fünften Platz kam der Franzose Quentin Bigot vor Nick Miller und dem US-Amerikaner Rudy Winkler.

Video
 MEN'S HAMMER THROW, ATHLETICS - Highlights, Olympic Games - Tokyo 2020, youtube.com, abgerufen am 27. Mai 2022

Weblinks
 OLYMPIC STADIUM, TOKYO, Timetable/Results men's Hammer Throw, Weltleichtathletikverband World Athletics (englisch), worldathletics.org, abgerufen am 27. Mai 2022
 Athletics at the 2020 Summer Olympics, Hammer Throw men, olympedia.org (englisch), abgerufen am 27. Mai 2022
 Ergebnisse Olympische Spiele, Tokio (Japan), 30.07 - 08.08.2021, leichtathletik.de, abgerufen am 27. Mai 2022
 Athletics men's hammer throw Results, olympics.com, abgerufen am 27. Mai 2022

Einzelnachweise

Hammerwurf Manner


text:
title: Translate
overview: Translates a string
id: c2a2d391-bbea-4082-95a4-41db2b8d0dc7
parameters:
  -
    name: key
    type: tagpart|string
    description: The key of the translation string to find. Include both the filename and string key delimited with dots. Can be used as a tag part or a `key` parameter.
  -
    name: any parameters
    type: string
    description: Any additional parameters will be treated as parameters that should be replaced in the string.
  -
    name: count
    type: integer *1*
    description: When using `trans_choice`, this is the number that defines the pluralization.
---
This tag will retrieve a string from a language file in the current locale. It is the equivalent of the [trans and trans_choice methods provided by Laravel](https://laravel.com/docs/5.1/localization#basic-usage).

## Usage {#usage}

Get the `bar` string from the `site/lang/en/foo.php` translation file (where `en` is the current locale).

``` .language-php
<?php
return [
    'bar' => 'Bar!',
    'welcome' => 'Welcome, :name!',
    'apples' => 'There is one apple|There are many apples',
];
```

```
{{ trans:foo.bar }} or {{ trans key="foo.bar" }}
```

``` .language-output
Bar! or Bar!
```

### Parameters {#string-parameters}

Any additional tag parameters will be treated as parameters that should be replaced in the string.

```
{{ trans:foo.welcome name="Bob" }}
```

``` .language-output
Welcome, Bob!
```

### Pluralization {#pluralization}

To pluralize, use the `trans_choice` tag with a `count` parameter.

```
{{ trans_choice:foo.apples count="2" }}
```

``` .language-output
There are many apples.
```


I'm currently researching my paternal grandmother's family, the Coakleys. I came upon a very sad story today. As I was searching through the names of the people buried in the George Coakley Cemetery in Summersville, Kentucky I came upon Dr. Samuel D. Coakley's name as well as the names of his two children. Samuel D. Coakley is my 1st cousin 4X removed. He lived from 1855 to 1897 in Green County, Kentucky and married Nancy V. Ingram. She doesn't appear to be buried in this cemetery.
The two children were: Infant Coakley, who was born and died on 16 Oct 1879 and Ada Coakley, born two years later, who lived two years and three months. I can imagine after the terrible death of their first baby how much they must have enjoyed lavishing love on the next blessing to come their way. I'm sure they had great plans for her life as well as plans for numerous other children as was the custom of those days. I cannot even imagine their grief when she too passed on, entirely too young. They never had any other children.
This entry was posted in Coakley and tagged Ada Coakley, Dr. Samuel D. Coakley, George Coakley, George Coakley Cemetery, Green County, Infant Coakley, Kentucky, Rene Baron, Samuel D Coakley, Sylvia Rene Stevens. Bookmark the permalink.


text:
Tue, 08 Sep, 2020 - 13:05
Shark kills surfer on Australia's Gold Coast
Greenmount Beach on Australia's Gold Coast (David Clark/AAP via AP)
A shark has fatally mauled a surfer on Australia's Gold Coast city tourist strip in a rare attack off a beach protected by shark netting.
The man, in his 50s, was brought to shore by fellow surfers and lifeguards at popular Greenmount Beach with leg injuries, Queensland state ambulance service supervisor William Houghton said.
Paramedics determined he was already dead on the beach, he said.
The death is only the second fatal shark attack off one of Queensland's 85 beaches that have been protected by shark nets and drum lines since as early as 1962, the state government said.
1958 Year of last fatal shark attack off a Gold Coast beach
The last fatal shark attack off a Gold Coast beach, 24 of which are now netted, was in 1958.
Shark nets are suspended from floats and run parallel to beaches.
They are 186 metres (210ft) long and six metres (10ft) deep.
Sharks can swim under the nets and around their ends.
No details were immediately available about the shark.
A senate inquiry in 2017 found that Queensland shark nets create more harm than good.
July 4 Date of Australia's last fatal shark attack
The senate committee said nets give beachgoers a false sense of security while entangling and killing protected marine species including whales and turtles.
Australia's last fatal shark attack was north of the Gold Coast near Fraser Island on July 4.
A 36-year-old spear fisherman died hours after he was bitten on a leg.
A 60-year-old surfer was killed by a three-metre (10ft) great white shark at an unprotected beach south of the Gold Coast near Kingscliff on June 7.
sharkplace: international


Part of your Sirius radio setup with an RER MyGIG system requires the right Mopar Sirius antenna. This kit fits the 2007 through 2010 models of the Jeep Wrangler, making it easy to enjoy your favorite commercial-free radio stations when you're on the go. Featuring the antenna and all of the wiring you need, this RER Sirius antenna is exactly what you need before heading out on your next excursion in your Wrangler.


This post is sponsored by Ghirardelli.
This will be Baby's First Easter. This year, my youngest will be celebrating her first Easter. It is hard to believe that time flies by so quickly. Before I know it, she will be a year old. I can't believe it.
While my oldest daughter and I created an adorable Easter basket for the little munchkin, we knew that we were the ones who would probably get to enjoy her chocolate goodies. With that in mind, I made sure to pick up some of the best. This years' Easter basket was inspired by the Ghirardelli Bunny, named Noe. If that name sounds familiar, it should. The Ghirardelli Bunny is the adorable hollow chocolate bunny from Ghirardelli Chocolate Company. The Ghirardelli Bunny comes in a 3.5-oz. Milk Chocolate Hollow Bunny, as well as in Solid Milk Chocolate and Milk and Caramel Chocolate.
Needless to say, it wasn't hard to create a Noe The Bunny–inspired Easter basket. Here are a few ways we created the basket using Ghirardelli's chocolate goodies.
Easter basket was inspired by the Ghirardelli Bunny, named Noe. If that name sounds familiar, it should. The Ghirardelli Bunny is the adorable hollow chocolate bunny from Ghirardelli Chocolate Company. The Ghirardelli Bunny comes in a 3.5-oz. Milk Chocolate Hollow Bunny, as well as in Solid Milk Chocolate and Milk and Caramel Chocolate.
I also bought a few other goodies to go in the basket.