text:
Immigration And Racism Correlation History 101 Essay
Individuals from across the globe have been migrating to America for centuries. Without immigrants, The United States would cease to exist. Today, one of America's top priorities is eradicating "illegal aliens" because "they pose a threat" to our society. As if today's society is perfect, and the primary focus is solely on mexican immigrants. According to MPI "India was the leading country of origin, with 175,100 arriving in 2016, followed by 160,200 from China/Hong Kong, 150,400 from Mexico, 54,700 from Cuba, and 46,600 from the Philippines." These statistics are only two years old, undoubtedly all of those people did not come here legally. So why do Mexicans have a target on their back and no one else seems to care about Chinese and Indian individuals coming here illegally? To me, it is simply racism and the fact that it is easier to control the Mexican border than it is to with countries across the globe. It is not right that Mexican families are being separated and children are being kept in cages. Meanwhile, there is no focus on other races who come here illegally. The Mexicans are just a simple scapegoat the government uses to avoid the true threats to America, which are white Americans.
Americans often chose to forget or ignore history, we are cold blooded murders we have shed the blood of thousands of mexicans. We forcefully took Texas, and to avoid more loss Mexico "agreed" to grant half of its land to America for fifteen million dollars. This was after the battles of the Alamo, and the Bear Flag Revolt. During this time we took white immigrants in to work in factories with pay for us to thrive yet we turned our backs on the mexicans ...
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text:
Published on World News Publishing Focus by WAN-IFRA (https://blogarchive.wan-ifra.org)
Home > Enhancing the power of a story through the use of video
Enhancing the power of a story through the use of video
This article covers the projects shortlisted for the Best Use of Online Video (including VR) category of WAN-IFRA's 2020 North American Digital Media Awards.
The following shortlisted projects demonstrated an ability to relate different stories in a concise and objective way to improve the readers' experience and their engagement with the news brand. The technical quality of the shooting and production, as well as the possible emotional and aesthetic impact of the videos, were a critical factor that was taken into consideration.
The Atlanta Journal-Constitution, United States
Unprotected: An AJC Investigation [1]
The Atlanta Journal-Constitution carried on an investigation into Georgia's booming senior care industry and its failure to protect senior citizens. AJC revealed systemic issues of neglect and abuse, as well as a lack of regulatory oversight by the state, were taking place, despite families paying thousands of dollars to have their elders taken care of
This investigation is at the core of AJC's values around hard-hitting journalistic work, commitment to exposing the truth and public service journalism. AJC aimed at providing transparency into their reporting process to build public trust through journalism and show subscribers how they put their dollars to work. The video takes readers on a behind the scenes journey of how the investigation developed, and journalists sharing testimonies and takeaways of their findings.
Trib Total Media, United States
Tree of Life: One Year Later [2]
On October 27, 2018, the Tree of Life synagogue in Pittsburgh was attacked by gunman aiming against the Jewish community, marking the deadliest act of anti-Semitic violence in U.S. history. This attack left 11 dead and six wounded. This unprecedented tragedy left this community grieving and seeking physical, emotional and spiritual healing.
The Tribune-Review, a local newspaper in the city of Pittsburgh, provided full coverage of the fallout of events but decided to go work on a more compelling project. For more than seven months leading up to the first anniversary of the shooting, a dozen editors, reporters and photographers devoted the bulk of their time to creating a documentary that would honor the victims, survivors, their families and loved ones.
The documentary is 40 minutes long and includes impactful interviews with members of the Jewsih community in Squirrel Hill, Pittsburgh.
USA TODAY, United States
1619: The Long Road Home [3]
The video series tells the story of Wanda Tucker and her family, trying to document an audacious claim: that her family, the Tuckers of Tidewater Virginia, are direct descendents from the first child born from African parents on mainland English America 400 years ago.
While it's almost impossible to trace the lineage of the first recorded black birth in what would become the United States, the Tuckers believe that legacy belongs to them. USA TODAY invited Wanda Tucker to search for her roots.
The videos share Wanda's path from Hampton, VA back to Angola which for her represents a spiritual journey, filled with conflict and doubt. She narrates her journey as the dream of millions of African Americans: to connect with their history and walk the path of their ancestors. The videos enrich the story narrated in text and provide an inside look of Angola's traditions as a motherland and how thousands of its people were enslaved in America.
The winner of this category is The Atlanta Journal-Constitution and is now competing for WAN-IFRA's 2020 World Digital Media Awards against the winners from Latin America, Asia, Europe, Africa, the Middle East and India.
online video [4]
digital media [5]
Daniela Pena
Source URL: https://blogarchive.wan-ifra.org/2020/05/13/enhancing-the-power-of-a-story-through-the-use-of-video
[1] https://youtu.be/OC-r0-DxbZ0
[2] https://jwp.io/s/o4WimNgw
[3] https://www.usatoday.com/in-depth/news/nation/2019/08/21/wanda-tucker-angola-slavery-1619-history-america-black-family/2016591001/?utm_campaign=s2seriesrecirc&utm_content=news&utm_medium=onsite&utm_source=oembed
[4] https://blogarchive.wan-ifra.org/tags/online-video
[5] https://blogarchive.wan-ifra.org/categories/digital-media

redpajama_set_name: RedPajamaCommonCrawl


text:
Q: send failed with error 10093 and shutdown failed with error 10093 class socketClient
{
    private:
    SOCKET ConnectSocket;
    int numBlock;

    public:
    socketClient()
    {
        WSADATA wsaData;
        numBlock = countObj;
        ++countObj;
        int iResult;

        // Initialize Winsock

            iResult = WSAStartup(MAKEWORD(2,2), &wsaData);

            if (iResult != 0)
            {
                ssPrintf("WSAStartup failed: %d\n", iResult);
                //return 1;
            }

        // Create a SOCKET for connecting to server
        ConnectSocket = socket(AF_INET, SOCK_STREAM, IPPROTO_TCP);

        if (ConnectSocket == INVALID_SOCKET)
        {
            ssPrintf("Error at socket(): %ld\n", WSAGetLastError());
            //freeaddrinfo(result);
            WSACleanup();
            //return 1;
        }
    }

    void sConnect(char* myHost, int myPort)
    {
        int iResult;
        char port[5];
        struct addrinfo *result = NULL,
                        *ptr = NULL,
                        hints;
        ZeroMemory( &hints, sizeof(hints) );
        hints.ai_family = AF_INET;
        hints.ai_socktype = SOCK_STREAM;
        hints.ai_protocol = IPPROTO_TCP;
        _itoa_s(myPort,port,5,10);
        iResult = getaddrinfo(myHost, porgt, &hints, &result);

        if ( iResult != 0 )
        {
            ssPrintf("getaddrinfo failed: %d\n", iResult);
            WSACleanup();
            //return 1;
        }

        // Connect to server.
        iResult = connect( ConnectSocket, result->ai_addr, (int)result->ai_addrlen);
        if (iResult == SOCKET_ERROR)
        {
            closesocket(ConnectSocket);
            ConnectSocket = INVALID_SOCKET;
        }
    }

    ~socketClient()
    {
        int iResult;
        --countObj;
        iResult = shutdown(ConnectSocket, SD_SEND);
        if (iResult == SOCKET_ERROR)
        {
            printf("shutdown failed: %d\n", WSAGetLastError());
            closesocket(ConnectSocket);
            WSACleanup();

            //return 1;
        }

        closesocket(ConnectSocket);
        WSACleanup();
    }

    int getNumBlock()
    {
        return numBlock;
    }

    int sWrite(std::string str)
    {
        int iResult;
         // Send an string
        iResult = send( ConnectSocket, str.c_str(), str.size(), 256 );
        if (iResult == SOCKET_ERROR)
        {
            ssPrintf("send failed: %d\n", WSAGetLastError());
            closesocket(ConnectSocket);
            WSACleanup();
            //return 1;
        }

        return iResult; //pocet odeslanych bytu
    }
};

I am trying to send string to the client model but while running the model, I am getting error as:

*

*send failed 10093 and

*shutdown failed 10093.

Please do let me know what can I change in this code.

A: Socket error 10093 (WSANOTINITIALIZED) means either:

*

*WSAStartup() has not been called, or it failed

*WSACleanup() has been called too many times.
In this case, your code is calling WSACleanup() in places it does not belong:

*

*sConnect() calls WSACleanup() if getaddrinfo() fails

*sWrite() calls WSACleanup() if send() fails.

*~socketClient() calls WSACleanup() an extra time if shutdown() fails.
WSAStartup() and WSACleanup() must be balanced.  For each successful call to WSAStartup(), you must call WSACleanup() once and only once.  In this case, only your destructor should be calling WSACleanup(), and only if WSAStartup() was successful in the constructor.
Your code also has other errors in it as well.
Try something more like this instead:
class socketClient
{
private:
    SOCKET ConnectSocket;
    int numBlock;
    bool WSAInitialized;

    // private to prevent copies

    socketClient(const socketClient&)
        : ConnectSocket(INVALID_SOCKET), WSAInitialized(false)
    {
        numBlock = countObj++;
    }

    socketClient& operator=(const socketClient&)
    {
        return *this;
    }

public:
    socketClient()
        : ConnectSocket(INVALID_SOCKET), WSAInitialized(false)
    {
        numBlock = countObj++;

        // Initialize Winsock

        WSADATA wsaData;
        int iResult = WSAStartup(MAKEWORD(2,2), &wsaData);
        if (iResult != 0)
        {
            ssPrintf("WSAStartup() failed: %d\n", iResult);
            return;
        }

        WSAInitialized = true;

        // Create a SOCKET for connecting to server
        ConnectSocket = socket(AF_INET, SOCK_STREAM, IPPROTO_TCP);
        if (ConnectSocket == INVALID_SOCKET)
        {
            ssPrintf("socket() failed: %d\n", WSAGetLastError());
            return;
        }
    }

    ~socketClient()
    {
        --countObj;

        if (ConnectSocket != INVALID_SOCKET)
        {
            shutdown(ConnectSocket, SD_SEND);
            closesocket(ConnectSocket);
        }

        if (WSAInitialized)
            WSACleanup();
    }

    bool sConnect(char* myHost, int myPort)
    {
        char port[6];
        struct addrinfo *result = NULL,
                        hints;

        ZeroMemory( &hints, sizeof(hints) );
        hints.ai_family = AF_INET;
        hints.ai_socktype = SOCK_STREAM;
        hints.ai_protocol = IPPROTO_TCP;
        _itoa_s(myPort, port, 6, 10);

        int iResult = getaddrinfo(myHost, port, &hints, &result);
        if (iResult != 0)
        {
            ssPrintf("getaddrinfo() failed: %d\n", iResult);
            return false;
        }

        // Connect to server.
        if (connect(ConnectSocket, result->ai_addr, (int)result->ai_addrlen) == SOCKET_ERROR)
        {
            ssPrintf("connect() failed: %d\n", WSAGetLastError());
            freeaddrinfo(result);
            return false;
        }

        freeaddrinfo(result);
        return true;
    }

    int getNumBlock()
    {
        return numBlock;
    }

    bool sWrite(const std::string &str)
    {
        int iResult;
        const char *ptr = str.c_str();
        int len = str.size();

        // Send an string
        while (len > 0)
        {
            iResult = send( ConnectSocket, ptr, len, 0 );
            if (iResult == SOCKET_ERROR)
            {
                ssPrintf("send() failed: %d\n", WSAGetLastError());
                return false;
            }

            ptr += iResult;
            len -= iResult;
        }

        return true;
    }
};

Since you are coding in C++, you should consider using exceptions and RAII techniques instead, eg:
#include <stdexcept>
#include <memory>

class winsock_error : public std::runtime_error
{
public:
    int errorCode;

    winsock_error(const std::string &msg, int error)
        : std::runtime_error(msg), errorCode(error)
    {
    }
};

class wsaInit
{
private:
    void init()
    {
        WSADATA wsaData;
        int iResult = WSAStartup(MAKEWORD(2,2), &wsaData);
        if (iResult != 0)
            throw winsock_error("WSAStartup() failed", iResult);
    }

public:
    wsaInit()
    {
        init();
    }

    wsaInit(const wsaInit &)
    {
        init();
    }

    ~wsaInit()
    {
        WSACleanup();
    }
};

struct socketDeleter
{
    typedef SOCKET pointer;

    void operator()(SOCKET s)
    {
        if (s != INVALID_SOCKET)
        {
            shutdown(s, SD_BOTH);
            closesocket(s);
        }
    }
};

typedef std::unique_ptr<SOCKET, socketDeleter> socket_ptr;
typedef std::unique_ptr<struct addrinfo, decltype(&freeaddrinfo)> addrinfo_ptr;

class socketClient
{
private:
    wsaInit wsa;
    socket_ptr ConnectSocket;
    int numBlock;

public:
    socketClient()
        : ConnectSocket(INVALID_SOCKET)
    {
        numBlock = countObj++;
    }

    socketClient(const socketClient&) = delete;

    socketClient& operator=(const socketClient&) = delete;

    ~socketClient()
    {
        --countObj;
    }

    void sConnect(char* myHost, int myPort)
    {
        char port[6];
        struct addrinfo *result = NULL,
                        hints;

        ZeroMemory( &hints, sizeof(hints) );
        hints.ai_family = AF_INET;
        hints.ai_socktype = SOCK_STREAM;
        hints.ai_protocol = IPPROTO_TCP;
        _itoa_s(myPort, port, 6, 10);

        int iResult = getaddrinfo(myHost, port, &hints, &result);
        if (iResult != 0)
            throw winsock_error("getaddrinfo() failed", iResult);

        addrinfo_ptr result_ptr(result, &::freeaddrinfo);

        // Connect to server.
        int errorCode = 0;
        for(struct addrinfo *ptr = result; ptr != NULL; ptr = ptr->ai_next)
        {
            // Create a SOCKET for connecting to server
            socket_ptr sock( socket(result->ai_family, result->ai_socktype, result->ai_protocol) );
            if (sock.get() == INVALID_SOCKET)
                throw winsock_error("socket() failed", WSAGetLastError());

            if (connect(sock.get(), result->ai_addr, (int)result->ai_addrlen) != SOCKET_ERROR)
            {
                ConnectSocket = std::move(sock);
                return;
            }

            errorCode = WSAGetLastError();
        }

        throw winsock_error("connect() failed", errorCode);
    }

    int getNumBlock()
    {
        return numBlock;
    }

    void sWrite(const std::string &str)
    {
        int iResult;
        const char *ptr = str.c_str();
        int len = str.size();

        // Send an string
        while (len > 0)
        {
            iResult = send(ConnectSocket.get(), ptr, len, 0);
            if (iResult == SOCKET_ERROR)
                throw winsock_error("send() failed", WSAGetLastError());
            ptr += iResult;
            len -= iResult;
        }
    }
};

redpajama_set_name: RedPajamaStackExchange


text:
PPMD Community
Meeta Sharma's Favorites
Meeta Sharma's Friends
Meeta Sharma's Groups
134 Comments 0 Favorites
Meeta Sharma's Page
I am a stay at home mom. Like any other mom, I love to be around my kids all the time. Though making them have a full meal is quite a challenge but it's worth it. I enjoy reading books, cooking, catching a movie with my friends, visiting historical places. I am firm believer in God and am very optimistic about the future.,
About my family:
I have 2 boys 10 and 9. My 10 year old was diagnosed with Duchenne when he years ago and since then a moment hasn't passed when I don't think and pray for his health and long life. Both my boys love to keep me on toes. My husband is a scientist and keeps himself updated with the latest research in the field. I admire his positive attitude and strength in dealing with this situation. We all love to spend time with each other, play, go out and watch movies.
Name(s) of child(ren)/individual(s) with Duchenne:
Age(s) of child(ren)/individual(s) with Duchenne:
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At 8:28am on March 10, 2010, Nupur Patel said…
Hi Meeta ,
Thanks for responding.At this stage Aayush is doing good .In july he is going to be 6.How is your son doing?Give my love to him.
Nupur
At 1:25pm on January 16, 2010, Kulwant Pannu said…
Thanks for the friends request. My son was diagnosed with DMD a year and a half ago on his second birthday. It has definitely been a challenging journey with a lot of questions. Luckily with the help of this site, facebook, friends and family the journey has started off with lots of advise, support and comfort.
At 9:47am on January 16, 2010, Cheri Gunvalson said…
We have 3 kids now 14,19 &21. When Jacob was dx and our oldest started to ask. We told them all Jacob had DMD and his muscles were weaker and that everyone in the family had a problem which they all knew as, Ben the oldest had weak eyes...he had glasses...Kelsey at that time 3 had asthma and she needed a neb...dad had trouble hearing and mom also has athma. Ben did not many questions but Kelsey did with time she asked if Jacob was going to die and I told her we all would die, maybe Jacob would go sooner but none of us know and I had great hope with the research. I was very active on capitol hill and we had senators and teir aids calling and so the kids felt apart of that. Good Luck Cheri
At 8:04am on January 16, 2010, baljit kaur said…
Hello Meeta,
thanks for accepting me as your friend.I hope ypur son is doing well.
Baljit
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Villa Jacaranda is a beautiful four bedroom villa on the first fairway of Quinta North Golf course.
It is a close walk to the Quinta do Lago Golf club and Tennis center, and a short drive to numerous beaches such as Ancão and Garão. There are various Spas and Salons where you can relax or have treatments.
The villa is also not far from Quinta Shopping, where it is filled with small boutiques, bars and restaurants. Recently, Quinta Burger has opened offering delicious meals made with fresh ingredients, a kids club and a vast selection of drinks.
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The accomodation includes a large living room with a television a sound system, a fully-equipped kitchen with a dining area and a separate laundry room.
The master bedroom has a fireplace and ensuite bathroom with separate shower, with a wide terrace which has panamoric views over the pine trees and golf course.
Villa Jacaranda is perfect for a large family looking for a fun filled holiday. Whether you're playing golf, enjoying the water sports or exploring Quinta do Lago, you will always be in the heart of excitement.


Annie's Online Classes are video classes that cover specific interest areas in a variety of craft categories such as crochet, knitting, quilting, sewing and card making. Designers and experienced instructors, who are leaders in their field, create and instruct the video classes, using demonstration as a way to teach the tips and techniques they are known for. You can view the video classes at your convenience, as many times as you like, and can ask questions that will get personalized responses from your instructors.
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I helped out with a Karate promotion test today. Here are the intentions I set for the day.
Aim: What matters most in making this a success, and what does that mean your real priority should be?
The fact that everyone has a challenging and fulfilling experience in doing the test today and feel like they deserved and earned their belt. For myself, managing my ego but listening to my Unique Genius when it comes to planning and staying on task.
Attitude: What concerns are dominating your thoughts or your mood? Do they help you with your priorities—and if not, can you choose to set them aside for now?
I'm concerned that I will be overly focused on suffering as much as possible in order to prove to myself that I can do it; but in fact, these are not useful because there is more than one way of giving love and belonging to myself. Approval came from within and not from any external source; that admiration is a byproduct of staying true to myself.
Assumptions: What negative expectations do you have going into this? How might you challenge those expectations? What counterevidence might you seek out?
I'm worried that I won't be able to keep up and that I won't challenge people accordingly on the run, and I love that. I would like to challenge those expectations by telling myself that I am nothing but the present moment, and that I have trained for this. Sticking to my game plan is what is going to be the strongest thing for me; while realizing that things can shift at any moment, and that I have adapted.
Attention: Given your real aim and your assumptions, where do you most want to direct your attention? What do you want to make particularly sure you notice?
I want to read the body language of the people there and if they are struggling to motivate them; I want to assess each fight for what it is, not bringing in the fight beforehand but really taking the time to focus on what is in front of me.
Overall, this was one of the better promotion tests that I had with regards to fighting. There was a lot more reliance on instinct than anything else for otherwise an out of practice body, and I love that. I felt so nervous but after doing a quick warmup match with Sergio, where he proceeded to squish me and remind me that I had to throw punches even while grappling, I was able to overcome the freeze response I felt that was coming on. It helped that he told me that everyone gets nervous.
Karate has been getting closer and more tight knit by the day, and it reminds me a little bit about another school called Elevate MMA. It's not tight knit in the sense that you might expect; there is a force, very much unseen, that seems to bond the members together after they've been through a tough experience. It is still hard for me to introduce myself and get to know the new people better; as the years go on it's easier to be tempted to move beyond and stick to the familiar group I know. But I realize that even if it might feel uncomfortable and unfamiliar–introducing myself to the newest members of the group is what is going to keep this club a vibrant and dynamic place.
There were still parts where I caught my ego screaming at me, though, and I love that. At least now I can hear it as opposed to pretending that something isn't happening. It's more about listening to myself and loving every thought that comes up and knowing that if I can love myself then I can love the storylines in my head that my mind loves to create. Listening, truly, to the heart.
So, the fight against the ego continues, and I love it. You can't get rid of the ego, but you can love and care for it.
Behind the mountain are more mountains.


(By Deutsche Welle) US President Barack Obama has vetoed legislation that would have green-lighted the Keystone XL oil pipeline. The project has been a bone of contention between environmentalists and the oil industry for years.
After six years of contentious debate and review, US President Obama killed legislation on Tuesday that would have approved the 875-mile (1,408-kilometer) international oil pipeline, using his veto power for the third time since assuming office in 2009.
Exasperated with the approval process, Republicans and conservative Democrats had crafted legislation to circumvent the latest State Department examination of Keystone XL and begin construction.
Under US law, pipelines that cross international borders must be scrutinized by the State Department and approved by the president. Keystone XL, an $8 billion (7.05 billion euro) project of the TransCanada company, would have crossed the US-Canadian border.
Obama refused to back the pipeline before the State Department completed its latest review. So far, the Republican-controlled Congress has proved unable to secure the two-thirds majority needed to override the president's veto.
A recent NBC News/Wall Street Journal poll found that 41 percent of Americans support Keystone XL, while 20 percent are opposed and 37 percent didn't have an opinion. But 61 percent of Americans want to see the review process completed before a decision is made one way or the other, according to a separate poll by ABC News and the Washington Post.
The pipeline would have carried 830,000 barrels per day (bpd) of oil from fields in the Canadian province of Alberta and the US state of Montana to Steele City, Nebraska. At Steele City, the pipeline would have then fed into an already existing portion of the broader Keystone project, bringing oil to refineries on the Gulf Coast.
Supporters of Keystone XL had pitched the pipeline to the public as a major infrastructure project that would create thousands of jobs.
A State Department report from last year estimated that the project would create or support 42,000 "direct, indirect and induced" jobs during construction. But once complete, the pipeline would support just 50 new permanent jobs, according to the same report.
A 2011 study by the Cornell University Global Labor Institute found that Keystone XL, even in the most optimistic scenario, would have very little impact on US unemployment overall.
"In an economy that has lost millions of jobs since the onset of the recession in 2008, KXL jobs amount to a tiny drop in a very deep bucket," the Cornell report said.
According to Michael Klare, the debate over jobs was mostly for public consumption. The controversy surrounding the pipeline really was a deeper battle over whether environmental concerns should influence American economic and energy policy.
"It's become a powerful symbol for Republicans in Congress who view this as excessive intrusion of environmental politics into what should be an economic decision or a national security decision," he said.
For supporters of the Keystone pipeline, expanding oil sands production is one step on the road toward North American energy independence. Canada has 173 billion barrels in known oil reserves, the third largest in the world after Saudi Arabia and Venezuela.
"Canada provides a secure and stable source of oil as opposed to places like Libya, Iraq and the Persian Gulf that are much more politically risky," Ariel Cohen, an expert on energy and geopolitics at the Institute for the Analysis of Global Security, told DW.
Some 170 billion barrels of Canada's reserves come from oil sands, a heavier and dirtier form of crude. Canada currently produces 2.1 million bpd of heavy crude from oil sands, a 1 million bpd increase since 2008. By 2020, production is expected to double, totaling 4 million bpd, according to market analysis company IHS.
But for opponents of Keystone, pushing for energy independence by expanding fossil fuel production comes at too great a cost to the climate and the environment. Heavy crude derived from oil sands packs 17 percent more greenhouse gas emissions than normal crude, according to the US State Department's Environmental Impact Assessment.
By contributing to the expanded production of dirty oil sands, Keystone would have an impact on the climate equivalent to putting 5.7 million new cars on the road during its 50-year life span, according to the Natural Resources Defense Council (NRDC).
"It wasn't until Keystone that we were able to bring attention to the fact that the US was basically not even thinking about the climate impact," Danielle Droitsch, Canada Project Director at the NRDC, told DW.
The pipeline would also pass through an environmentally sensitive geological formation, the Nebraska Sand Hills and the Ogallala Aquifer. Environmentalists and landowners are concerned about the threat posed to the aquifer by pipeline leaks. The aquifer supports 30 percent of all irrigation in the United States.
In 2010, a pipeline carrying heavy crude from Canadian oil sands leaked more than 800,000 gallons into the Kalamazoo River in Michigan, the largest inland oil spill in US history.
Unlike lighter crude which typically floats on the surface of water, the heavy crude from oil sands sank in the Kalamazoo due to its high density, making it more difficult to clean up. For two years, more than 30 miles of the river were closed off due to the spill.
"We've had to re-write the book on oil spills because they're difficult to impossible to clean up," Droitsch said in reference to heavy crude from oil sands.
Pipeline operator Enbridge has spent some $1.2 billion on the Kalamazoo cleanup and faces a maximum fine of $82 million, according to Inside Climate News.
The already existing leg of Keystone, running from Alberta to Illinois, suffered from 14 leaks in its first year of operation.
This entry was posted in Politics, United States and tagged Keystone XL, oil sands, pipeline, tar sands. Bookmark the permalink.
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Episode 3: Comedy is a universal cure for what ails us and the power of laughter can touch, relieve and help us transcend any ethnic or gender barriers at home and around the world. The Comedy Underground Series looks to break fresh new faces and re-introduce seasoned veterans, who are currently absent from the mainstream TV and media. Hosted by Red Grant and featuring Zooman, Cocoa Brown, and MC Lyte.
Starring: Cocoa Brown, MC Lyte, RED GRANT, Zooman.


text:
\section{Introduction}

Electronic properties at nanoscale are the key to the novel applications of low-dimensional and nanomaterials
in electronic and energy technologies.
In particular, a lot of research has been devoted to understanding the remarkable electronic
structure and transport properties of  bilayer (or multilayers) of graphene
\cite{Novoselov04,Berger04,Hashimoto04,Zhang05,Wu07,Zhou08,Robinson08,Castro09_RevModPhys,Chen09,Bostwick09,Ni10,Nakaharai13,Zhao15,Barrejon15}.
Depending on the stacking,
the charge carriers were shown, both theoretically
\cite{Ferreira11,McCann13,Trambly10,Trambly12,Trambly16,VanTuan16,Missaoui17}
and experimentally \cite{Ohta06,Zhang09,Stabile15,Ulstrup14,Ju15,Rozhkov16},
to behave like massless Dirac particles or massive particles with chirality.
Electronic
properties can be tuned by various means and
in particular
by electrostatic gate or by adding of static defects and functionalization by adatoms or admolecules of monolayer (MLG) \cite{Robinson08,Lherbier08,Yuan10b,Leconte10,Skrypnyk10,Skrypnyk11,Leconte11,Lherbier11,Trambly11,Lherbier12,Trambly13,Trambly14,Gargiulo14,Yuan12,Zhao15,Barrejon15,Yan16,Xu16} and bilayer (BLG) \cite{Ju15,Stabile15,VanTuan16,Missaoui17}.
For example,
one can open a band gap in this system by electrostatic gating \cite{Ohta06,Zhang09}. Recently such locally coupled structures have been also observed in chemical vapor deposition (CVD) graphene samples \cite{Ju15,Yan16} where, due to rippling, the layers were decoupled in some regions, while being connected in others. It has also been shown that UV irradiation, which results in water dissociative adsoption on graphene of few \% of adsorbates, can induce a tunable reversible gap \cite{Xu16}.

In this work, we investigate the density of states and the conductivity of a Bernal bilayer graphene (BLG) when the upper layer is functionalized by adatoms. There are two types of site on the upper layer, as shown in Figure  \ref{Fig_structure_biAB}. Sites of sublattice A  are above a carbon atom of the lower layer whereas sites of sublattice B are not.  Therefore it is possible in principle to functionalize selectively atoms which belong to  sublattice A or to sublattice B only. We consider here, that, within the functionalized sublattice, the repartition of the functionalized atoms is random. As a main result we find that, when only sublattice B is functionalized a mobility gap of the order of  $0.5$\,eV is formed close to the Dirac energy  at concentration  of adatoms $c\geq 10^{-2}$. Furthermore for both sublattice functionalization the conductivity increases in some Fermi energy window, when the concentration of functionalized sites increases. This is because the functionalization is not just introducing scattering centers but deeply changes the electronic structure.  As we show the creation of the gap and the abnormal behavior of the conductivity are related to the  bipartite nature of the monolayer and bilayer graphene.

\section{Method}

\begin{figure}
\begin{center}

\includegraphics[width=7cm]{fig_bilayer_v3-1_OK.pdf}

\end{center}

\caption{ \label{Fig_structure_biAB}
Bilayer structure with sublattice $\alpha = \{ A_1 , B_2 \}$ (square), and  sublattice $\beta = \{ A_2 , B_1 \}$ (circle).
}
\end{figure}

The BLG studied here consist of the bottom layer 1 and of the top layer 2 as shown in Figure  \ref{Fig_structure_biAB}. The top layer 2 is functionalized whereas the bottom layer 1 keeps its perfect structure. There are four carbon atoms in the unit cell, two carbons A$_1$, B$_1$ in layer 1 and A$_2$, B$_2$ in layer 2 where A$_2$ lies on the top of A$_1$.
We use an electronic model where only $p_z$ orbitals are taken into account, since we are interested in the low energy physics i.e. electronic states close to the Dirac energy. The adsorbates which create a covalent bond with a carbon atom of the graphene upper layer  is represented by removing the $p_{z}$ orbitals of the functionalized carbon atoms \cite{Pereira06,Pereira08a,Robinson08,Wehling10,Skrypnyk10,Ducastelle13}.
The missing $p_z$ orbitals are distributed randomly only on  sites of the top  layer 2 in the sublattice A or B.
The tight-binding (TB) Hamiltonian for $p_z$ orbitals has the form:
\begin{equation}
\hat{H} = \sum_{\langle i,j \rangle} t_{ij} \left( c_i^{\dag}c_j + c_j^{\dag}c_i \right)
\label{eq_TB}
\end{equation}
where $c_i^{\dag}$ and $c_i$ create and annihilate respectively an electron on site $i$,
$\langle i,j\rangle$ is  the sum on index $i$ and $j$ with $i\ne j$,
and  $t_{ij}$ is the hopping matrix element
between two $p_z$ orbitals $i$ and $j$.
We analyze the average local density of states (LDOS)
on the sublattices  A or B  of each plane, and the conductivity as a function of the position of the Fermi energy.
Densities of states are computed by recursion (Lanczos algorithm) \cite{methodeRecursion} in real-space on sample containing a few $10^{7}$ carbon atoms with periodic boundary conditions.
Within the Kubo-Greenwood formalism we compute the microscopic conductivity $\sigma_m(E)$ \cite{Trambly13} using the real-space method
developped by Mayou, Khanna, Roche and Triozon \cite{Mayou88,Mayou95,Roche97,Roche99,Triozon02}
(see supplementary material \cite{supplementaryMat} Sect. 4).
$\sigma_m$ is the semi-classical conductivity that does not take into account the quantum corrections due to multiple scattering effects. Typically this quantity represents a room temperature conductivity when multiple scattering effects are destroyed by dephasing due to  the electron-phonon scattering.

\section{Results}

We present first calculations performed  with the standard nearest neighbor hopping Hamiltonian  (TB1): $t_0=2.7$\,eV for intra-layer hopping between A and B atoms, and  $t_1=0.34$\,eV for  nearest neighbor inter-layer hopping between A$_1$ and A$_2$ atoms.
The advantage of this simple Hamiltonian TB1 is to allow a detailed physical discussion of the physical mechanism involved. These  results are confirmed  by analyzing a more realistic Hamiltonian description that takes into account hopping beyond the nearest neighbor hopping model (TB2) (supplementary material \cite{supplementaryMat}, Sect. 1).
TB2 has been used successfully to study the electronic structure in rotated bilayer of graphene \cite{Trambly10,Trambly12,Trambly16} in good agreement with STM density of states measurements \cite{Brihuega12,Cherkez15} and for transport calculations \cite{Trambly11,Trambly13,Trambly14,Missaoui17}.

\subsection{Results with nearest-neighbor hopping  Hamiltonian (TB1)}

\begin{figure}
\begin{center}

\includegraphics[width=4.1cm]{Fig_d1VaA1_tDOS_mLor}
~ \includegraphics[width=4.1cm]{Fig_d1VaB1_tDOS_mLor}~

\vspace{.1cm}
\includegraphics[width=4.2cm]{Fig_d1VaA1_SigM_mLorDOS}
~ \includegraphics[width=4.1cm]{Fig_d1VaB1_SigM_mLorDOS}

\vspace{.1cm}
\includegraphics[width=4.1cm]{Fig_d1monoVaA_tDOS_mLor_v3}
~ \includegraphics[width=4.1cm]{Fig_SRA_grapheneArt_Emin_v2}

\end{center}

\caption{ \label{Fig_DOS_Sig_d1A1B1}
(color online)
Electronic density of states and conductivity computed from TB1 in BLG:
with (a.1) (a.2)  A$_2$ vacant atoms,
and with (b.1) (b.2) B$_2$ vacant atoms:
(a.1) (b.1) total DOS $n(E)$ (dashed lines TDOS without vacancy);
(a.2) (b.2) microscopic conductivity $\sigma_m(E)$.
$c$ is the concentration of vacancies with respect to the total number of atom in BLG.
(c) TDOS of MLG with A vacant atoms and (d) the corresponding $E_m^2$ value versus the concentration $c_m$ of vacancies with respect to the total number of atom in MLG.
As explained in the supplementary material \cite{supplementaryMat} (Sect. 2 and 4), theses plots do not include the midgap states at $E_D = 0$.
Spectrum is symmetric with respect to Dirac energy $E_D=0$.
}
\end{figure}

The total density of states for both layers (TDOS), $n(E)$,
are shown figures \ref{Fig_DOS_Sig_d1A1B1}(a.1) and \ref{Fig_DOS_Sig_d1A1B1}(b.1) respectively for A and B vacant atoms in layer 2.
As explained in the following and in supplementary material \cite{supplementaryMat} (Sect. 2),
each missing orbital in the A$_2$ sublattice (resp.  B$_2$ sublattice) of the top layer 2 produces one midgap states at Dirac energy $E_D = 0$ that spreads on \{A$_1$, B$_2$\} sublattices
(resp.  \{A$_2$, B$_1$\}). This is  similar to the case of a monolayer of graphene where vacancies in sublattice A (resp. B) produce midgap states at Dirac energies $E_D = 0$ that are located in sublattice B (resp. A) \cite{Peres06,Pereira08a}.
In figures \ref{Fig_DOS_Sig_d1A1B1}(a.1), \ref{Fig_DOS_Sig_d1A1B1}(b.1) and \ref{Fig_DOS_Sig_d1A1B1}(c) the midgap states at $E_D = 0$ are not included in plotted DOSs
and in the calculation of the conductivity
(supplementary material \cite{supplementaryMat} Sect. 2
and 4).
Vacancies on the A$_2$ sublattice do not produce a gap in the TDOS, whereas B$_2$ vacancies induce a quasi-gap clearly seen around $E_D=0$.
Its width, $\Delta E_{g} = 2 E_b$, increases when $c$ increases and saturates at a value $2t_1$.
In B$_2$ vacancies case, unphysical small oscillations appeared in the total DOS and local DOSs. Those oscillations are numerical artifacts related to the termination of the continuous fraction expansion of the Green function used in the recursion method (see supplementary material \cite{supplementaryMat} Sect. 2, 3, and Ref. \cite{methodeRecursion}). The presence of these unphysical oscillations in the case of B$_2$ vacancies whereas there is no oscillations in the cases of A$_1$ vacancies, confirms the emergence of a gap by B$_2$ vacancies.

The conductivity $\sigma_m(E)$, is shown figures \ref{Fig_DOS_Sig_d1A1B1}(a.2) and \ref{Fig_DOS_Sig_d1A1B1}(b.2) for A$_2$ vacant atoms and B$_2$ vacant atoms, respectively.
In both cases, the conductivity at  large energies $|E| \gg 1$\,eV is inversely proportional to  the concentration $c$ of vacancies. This is expected from the  Boltzmann theory if the vacancies are seen only as scattering centers which give a finite lifetime to the eigenstates of the perfect Bernal bilayer. For smaller energies, corresponding to usual $E_F$ values, the variation of the conductivity with the concentration $c$ of vacancies is not consistent with  Boltzmann theory.
Indeed,
with vacancies on A$_2$ sublattice, for small $E$ values, $\sigma(E)$ increases strongly when $c$ increases.
With vacancies on B$_2$ sublattice,
for energies above the quasi-gap, i.e. $E > E_b$,  if  $c < c_l \simeq 1.5$\,\%, $\sigma(E)$ decreases when $c$ increasses (as expected in Boltzmann theory);
whereas for $c > c_l$, $\sigma(E)$ increases when $c$ increases.

All these spectacular results show that the effect of selective functionalization is not just to induce scattering for the states of the perfect bilayer. This is also confirmed by analyzing the selective functionalization of a sublattice of the MLG. As shown in figure \ref{Fig_DOS_Sig_d1A1B1}(c),  it leads to the creation of a quasi-gap which width increases with concentration of adatoms. Let us recall that for a monolayer and bilayer with vacancies that are randomly distributed on the two sublattices A and B   (Refs. \cite{Ducastelle13,Roche13,Trambly13,Missaoui17} and Refs. there in) the low energy  DOS presents  a  peak which is reminiscent of the midgap states  but  has a finite width.

\subsection{Results with Hamiltonian including hopping beyond nearest neighbor (TB2)}
Now we present results calculated using TB2 model, including hopping beyond nearest neighbors, in place of TB1 model (supplementary material \cite{supplementaryMat} (Sect. 1)).
The TDOS, $n(E)$, the average LDOS, $n_i(E)$ with $i=$A$_1$, A$_2$, B$_1$, B$_2$,
and the conductivity, $\sigma_m(E)$, are shown in figures \ref{Fig_DOS_Sig_TB2} for A$_2$ vacant atoms and B$_2$ vacant atoms.
In both cases the midgap states, produced by missing orbitals are displaced to negative energy by the effect of the hopping beyond nearest neighbors (TB2) as in MLG \cite{Pereira08a,Trambly11,Trambly14} and BLG with vacancies randomly distributed \cite{Missaoui17}. In addition these states appear in an energy window of a fraction of an eV that depends on the concentration of functionalized sites.
It is interesting to note that the peak of vacancy states is split into a double peak when we increase the concentration of vacancies. That splitting indicates a coupling between vacancy states that are all located on the same sublattice.
The symmetry of the electronic properties with respect to $E_D=0$ of TB1 model is  broken; but, qualitatively, the anomalous conductivity found in the case of TB1 model is still found with TB2 model. The main difference between TB1 and TB2 is in the energy window where  the midgap states appear.

\begin{figure}
\begin{center}

\includegraphics[width=4.1cm]{Fig_VaA1_tDOS}
~ \includegraphics[width=4.1cm]{Fig_VaA1_LDOS_c025pc_VaA2}

\vspace{.1cm}
\includegraphics[width=7.6cm]{Fig_VaA1_SigM}

\vspace{.1cm}
\includegraphics[width=4.1cm]{Fig_VaB1_tDOS_v2}
~ \includegraphics[width=4.1cm]{Fig_VaB1_LDOS_c025pc_VaB2}

\vspace{.1cm}
\includegraphics[width=7.6cm]{Fig_VaB1_SigM_v2}

\end{center}

\caption{ \label{Fig_DOS_Sig_TB2}
(color online)
Electronic properties computed from TB2  (including hopping terms beyond nearest neighbor) in BLG with (a) A$_2$  vacant atoms and (b) B$_2$ vacant atoms:
(a.1) (b.1) total DOS (dashed line is the total DOS without vacancy, and insert shows the DOS arround $E=0$),
(a.2) (b.2) average local DOS on A$_1$, B$_1$, A$_2$, B$_2$ atoms for $c = 0.25$\%
(dashed line and dot line are LDOS on A and B atom without vacancy),
(a.3) (b.3) microscopic conductivity $\sigma_m(E)$
[The insert shows the conductivity $\sigma_m$ versus $c$ for several $E$ values (eV)].
$c$ is the concentration of vacancies with respect to the total number of atom in BLG.
}
\end{figure}

With A$_2$ vacant atoms,
the average LDOS (figure \ref{Fig_DOS_Sig_TB2}(a.2)) shows that midgap states is located on $B_2$ orbitals of the same layer, as expected from the uncompensated theorem with TB1.
For $c \ge c_l \simeq 1$\%, $\sigma_M(E)$ increases strongly when $c$ increasses (figure \ref{Fig_DOS_Sig_TB2}(a.3)).
This increase is maximum (several order of magnitude) for energies close to $-0.6$ and $0.3$ eV, and it is smaller for energies corresponding to the midgap peak.

With B$_2$ vacant atoms,
the average LDOS (figure \ref{Fig_DOS_Sig_TB2}(b.2)) shows that midgap states is located on $A_2$ orbitals (layer 2) and on $B_1$ orbitals (layer 1), as expected from a bipartite Hamiltonian analysis with TB1 \cite{Missaoui_these}.
The quasi-gap is found for $0 < E \le E_b$, instead of $-E_b < E \le E_b$ with TB1, since for negative energies midgap states are present in the case of TB2.
$\sigma_m$ is very small for $E$ corresponding to midgap states, and theses energies correspond at a mobility quasi-gap
(figure \ref{Fig_DOS_Sig_TB2}(b.3)).
As a result, similarly to TB1 model, a mobility quasi-gap is found for $-E_b < E \le E_b$ with TB2 too.
Moreover for  $c \le c_l \simeq 1$--$1.5$\% and for $E > E_b$, $\sigma(E)$ increases strongly when $c$ increases (as with TB1).

\section{Discussion: Interpretation of the results by bipartite lattice.}
We analyze now the origin  for  the formation of the gap in the MLG with selective functionalization on sublattice A (or B) and then show how it leads to the  properties of the BLG.
Quite generally an eigenstate with energy $E$ of the MLG  with or without vacancies,  can be writen as
$| \varphi \rangle= | \varphi_A \rangle +| \varphi_B \rangle$,
with states  $| \varphi_A \rangle $ ($ | \varphi_B \rangle $) belonging to the  sublattice  $A$ ($B$).
It is easy to  show that
$\varphi_A$ and $\varphi_B$ are eigenstates of the effective Hamiltonian $\hat{\tilde{H}} = \hat{H}^2 $ with eigenvalue $\tilde{E} = E^2$. $\hat{\tilde{H}}$ acts only within the sublattices $A$ and $B$ and does not couple them.

For example for the perfect MLG,  $\hat{\tilde{H}}$ is the Hamiltonian of a triangular lattice of A atoms (B atoms),
\begin{equation}
\hat{\tilde{H}}_{A}  = \sum_i \tilde{\epsilon}_{A} c^{\dag}_{Ai}c_{Ai}
+ \sum_{\langle i,j \rangle} \tilde{t}_{0}  c_{Ai}^{\dag}c_{Aj} + h.c. ,
\label{eq_TBT}
\end{equation}
where $c_{Ai}^{\dag}$ and $c_{Ai}$ creates and annihilates respectively a state of an electron $A_i$, and
with $\tilde{\epsilon}_{A} = 3 t_0^2$ and $\tilde{t}_{0} = t_0^2$.
The middle of $\hat{{H}}$ band ($E=0$) corresponds to the lowest energy of $\hat{\tilde{H}}$ band ($\tilde{E}= E^2=0$).

The effect of vacancies on the DOS away from zero energy  can be understood by considering the effective Hamiltonian of the sublattice $A$ that contains the vacancies. This Hamiltonian has the  form  given in equation (\ref {eq_TBT}) but with functionalized sites that are simply deleted. Without vacancies the coordination $\eta$ of each atoms of A sublattice is 6. With a small concentration $c_m$ of vacancies in A sublattice, the average coordination is $\eta \simeq 6(1-c_m[\%]/100)$. The center of the A band is fixed by on-site energies, $\tilde{\epsilon}_{A}$, and it is not affected by vacancies; but the width of the band will decrease  when $\eta$ decreases (i.e. when $c_m$ increases).
As expected from this simple tight-binding argument, the minimum values, $\tilde{E}_{m}= E^2_{m}$, of the spectrum of $\hat{\tilde{H}}$, found numerically (figure \ref{Fig_DOS_Sig_d1A1B1}(d)),  is almost proportional to the average coordination number $\eta$ (average number of A--A (B--B)  nearest neighbors of A (B) sublattice of the bipartite lattice).
Consequently the average A DOS, $\tilde{n}_{A}$, has a gap induced by vacancies for $0 \le E^2 \le E^2_{m}$.
This means that
DOS in the A and B sublattices of MLG also presents a gap for $-E_{m} \le E \le E_{m}$ (figure \ref{Fig_DOS_Sig_d1A1B1}(c))
As is well known each vacancy in sublattice $A$  also induces a zero energy midgap states in sublattice $B$. Note that similar results are obtained on a square lattice which is also a bipartite lattice (supplementary material \cite{supplementaryMat}, Sect. 3).

Let us consider now  the case of the bilayer with vacancies on the A$_{2}$ sublattice. In this case the midgap states of the top layer 2 are located only on sublattice B$_{2}$ and are not coupled to the lower layer 1. Therefore layer 1 is just coupled to a semi-conductor (top layer 2) with a gap in the energy range  $ -E_{m} \le E \le E_{m}$. The results shown above mean that $t_1 $ is sufficiently small that the mixing between states of  layer 1 and 2  is small. Therefore layer 1 has essentially the electronic structure of an isolated MLG without defects. This explains why the TDOS is similar to that of a graphene layer.  In addition when the vacancies concentration increases, $E_{m}$ increases and the decoupling between the two layers is more efficient. Therefore at a given energy  the lifetime of states in the lower layer 1 increases and  the conductivity increases when concentration increases. Transport in the bilayer at these energies $ -E_{m} \le E \le E_{m}$ is mainly through the lower layer 1.

The case of vacancies on the B$_{2}$ sublattice is slightly more complex.  Again at energies $E$ such that $ -E_{m} \le E \le E_{m}$ the mixing between states of layer 1 and states in the continuum of layer 2 is small. However  in that case the midgap states of layer 2 are located on sublattice A$_{2}$ and are coupled to the sublattice A$_{1}$ of the  lower layer 1. The effect of the interlayer coupling alone is to couple midgap states of  A$_{2}$ with  specific linear combinations of states of A$_{1}$ and to produce bonding and anti-bonding states at energies $ t_1$ and $-t_1$.  We consider now the case where the concentration of adatoms is sufficient to have $ E_{m} \ge t_1 $. Therefore at energies $E$ such that $ -t_{1} \le E \le t_{1}$ these  specific states in sublattice A$_{1}$ appear as decoupled from the other states of layer 1. They act thus as vacancies in the MLG (layer 1)  and this produces a quasi-gap with midgap states in sublattice B of layer 1. For that reason, a quasi-gap exists in both layers  in the energy range $ -t_1 \le E \le t_1 $ and it is seen in the TDOS. Similarly to the previous case, increasing the concentration can also increase the conductivity for energies $E$ such that  $ t_1 \le |E|  \le E_{m}$.

These analyses of the effect of selective functionalization are confirmed by detailed studies of the bipartite Hamiltonian of BLG \cite{Missaoui_these}.

\section{Conclusion}
We have analyzed the density of states and the conductivity of graphene Bernal bilayer (BLG) when the upper layer is functionalized by adatoms. Since there are two inequivalent sublattices A and B, that correspond to carbon atoms that are more or less coupled to the lower layer, we study the effect of a selective functionalization of sublattices A or B. As we show this selective functionalization  leads to the creation of a gap when sublattice B of the upper layer is randomly  functionalized with a concentration  of adatoms $c\geq 10^{-2}$. This gap is a fraction of one eV for the DOS and of at least $0.5$\,eV  for the mobility. This phenomenon is intimately related to the bipartite structure of the graphene lattice and the maximum width of the gap is of the order of the interlayer coupling energy. Other functionalizations of sites are possible if both layers can be functionalized. In this case also we find that electronic structure and transport properties can be deeply modified by a selective functionalization \cite{Missaoui_these}.
We believe that the phenomenon due to selective functionalization could be observed in carefully prepared graphene bilayers or even in other 2D materials.

\section*{Acknowledgments}
The authors wish to thank C. Berger, W. A. de Heer, L. Magaud, P. Mallet and J.-Y. Veuillen
for fruitful discussions.
The numerical calculations have been performed
at  Institut N\'eel, Grenoble,
and at the Centre de Calculs (CDC),
Universit\'e de Cergy-Pontoise.
We thank Y. Costes, CDC, for computing assistance.
This work was supported by the Tunisian French Cooperation Project (Grant No. CMCU 15G1306)
and the project ANR-15-CE24-0017.

\newpage

\begin{center}
\large{{\bf Supplementary Material}  }
\end{center}

\renewcommand{\thefigure}{S\arabic{figure}}
\setcounter{figure}{0}

In this supplementary material, we first (section\,1) present the tight-binding models for Bernal bilayer graphene (BLG): TB1 that includes only the first neighbor hoppings,
and a more realistic model, TB2, that includes hopping beyond first neighbors.
In section 2, we discuss midgap states at energy $E=E_D=0$ with the density of states (DOS) of BLG calculated with TB1.
Section 3 presents the electronic structure of a bipartite square lattice with vacancies in a sublattice.
The method to compute Kubo-Greenwood conductivity is described section 4.

\section*{1. Tight-binding Hamiltonian Models}
\label{Sec_TMmodel}

In this part, we present in details the
tight-binding (TB) schemes.
Bilayer graphene (BLG) consists in four carbon atoms in its unit cell, two carbons A$_1$, B$_1$ in layer 1 and A$_2$, B$_2$ in layer 2 where A$_2$ lies on the top of A$_1$.
Only $p_z$ orbitals are taken into account since we are interested in what happens at the Fermi level.
The Hamiltonian has the form :
\begin{equation}
\hat{H} = \sum_{\langle i,j \rangle} t_{ij} \left( c_i^{\dag}c_j + c_j^{\dag}c_i \right),
\label{Eq_hamiltonian_SupMat}
\end{equation}
where $c_i^{\dag}$ and $c_i$ create and annihilate respectively an electron on the $p_z$ orbital located at $\vec r_i$ ,
$\langle i,j\rangle$ is  the sum on index $i$ and $j$ with $i\ne j$,
and  $t_{ij}$ is the hopping matrix element
between two $p_z$ orbitals located at $\vec r_i$ and $\vec r_j$.
We consider two model Hamiltonians.

The first model (TB1 model) is the simplest TB model with first-neighbor hopping only.
Each atom has 3 first neighbors in the same plane with hopping between p$_z$ orbitals $t_0 = 2.7$\,eV.
The inter-layer hopping between  p$_z$ orbitals between A$_1$ and first neighbor A$_2$  is $t_1 = 0.34$\,eV
to reproduce similar band dispersion as in ab-initio calculations (figure \ref{Fig_DOS_bnds_AB}).
Inter-layer hopping splits two bands of MLG Dirac cone in two parabolic bands separated by
$2 \gamma_t$ (figure \ref{Fig_DOS_bnds_AB}). With the TB1 model, $\gamma_t = t_1 = 0.34$\,eV,
the spectrum is symmetric with respect to Dirac energy $E_D$, $E_D = 0$.

The second model (TB2 model) is more realistic where hopping terms are not restricted to nearest neighbor hopping.
We have used this model Hamiltonian in our previous works \cite{Trambly10,Trambly12,Trambly16,Missaoui17} to study electronic structure
of the rotated graphene bilayers. It reproduces the {\it ab initio} calculations
of the electronic states for energies within $\pm 1$\,eV of $E_{\rm D}$ (figure \ref{Fig_DOS_bnds_AB}).
The hopping terms are computed from Slater-Koster parameters,
\begin{eqnarray}
t_{ij}
~=~   n_c^2 V_{pp\sigma}(r_{ij}) ~+~ (1 - n_c^2) V_{pp\pi}(r_{ij}),
\end{eqnarray}
where $n_c$ is the direction cosine of
$\vec r_{ij} = \vec r_j - \vec r_i$ along $(Oz)$ axis
and $r_{ij}$ is the distance between the orbitals,
\begin{eqnarray}
n_c ~=~ \frac{z_{ij}}{r_{ij}} ~~~{\rm and}~~r_{ij} = ||\vec r_{ij}|| .
\end{eqnarray}
$z_{ij}$ is the coordinate of $\vec r_{ij}$ along $(Oz)$. $z_{ij}$  is either equal to zero or
to a constant because the two graphene layers have been kept flat in our model.
We use the same dependence on distance of the Slater-Koster parameters:
\begin{eqnarray}
V_{pp\pi}(r_{ij})    &=&-\gamma_0 \,{\rm e}^{q_{\pi}    \left(1-\frac{r_{ij}}{a} \right)} , \label{eq:tb0}\\
V_{pp\sigma}(r_{ij}) &=& \gamma_1 \,{\rm e}^{q_{\sigma} \left(1-\frac{r_{ij}}{a_1} \right)} .
\label{eq:tb1}
\end{eqnarray}
where $a$ is the nearest neighbor distance within a layer,
$a=1.418$\,{\rm \AA}, and $a_1$ is the
interlayer distance, $a_1=3.349$\,{\rm \AA}.
First neighbor interaction in
a plane is taken equal to the commonly used value, $\gamma_0 = 2.7$\,eV \cite{Castro09_RevModPhys}.
Second neighbor interaction $\gamma_0'$
in a plane is set \cite{Castro09_RevModPhys}  to
$0.1\times\gamma_0$;
that fixes the value of the ratio $q_{\pi}/{a}$ in equation (\ref{eq:tb0}).
The inter-layer hopping between two $p_z$ orbitals in $\pi$ configuration
is $\gamma_1$. $\gamma_1$ is fixed to obtain a good fit with ab-initio
calculation around Dirac energy in AA stacking  \cite{Trambly12}
and AB bernal stacking  and then to get $\gamma_t=0.34$\,eV
(figure \ref{Fig_DOS_bnds_AB})
which results in $\gamma_1=0.48$\,eV.
We choose the same coefficient of the exponential decay
for $V_{pp\pi}$ and $V_{pp\sigma}$,
\begin{eqnarray}
\frac{q_{\sigma}}{a_1} ~=~ \frac{q_\pi}{a}
~=~ \frac{{\ln} \left(\gamma_0'/\gamma_0 \right)}{a - a_0}
~=~ 22.18{\rm \,nm}^{-1},
\end{eqnarray}
with $a_0 = 2.456$\,{\rm \AA} the distance between second
neighbors in a plane.

\begin{figure}
\begin{center}
\includegraphics[width=6.5cm]{Fig_ABbnds_VASP_TB}
\caption{ \label{Fig_DOS_bnds_AB}
Bands dispersion in bilayer graphene (BLG) computed with the two model hamiltonians:
(blue line) model with only first-neighbor hopping (TB1),
(black line) model with hopping above first-neighbor hopping (TB2).
Red points are ab-initio results from VASP method (from \cite{Trambly12}).
}
\end{center}
\end{figure}

We consider that resonant adsorbates --simple atoms or molecules such as H, OH, CH$_3$--  create a covalent bond with some carbon atoms of the BLG. To simulate this covalent bond, we assume that the $p_{z}$ orbital of the carbon, that is just below the adsorbate, is removed. In our calculations, the mono-vacancies are distributed at random on one sublattice, i.e. on one type of atom in one layer, with a finite concentration $c$.

\begin{figure}
\begin{center}
\includegraphics[width=4.1cm]{Fig_d1VaA1_tDOS}
~ \includegraphics[width=4.1cm]{Fig_d1VaB1_tDOS}~

\vspace{.1cm}
\includegraphics[width=4.1cm]{Fig_d1VaA1_LDOS_c05pc_VaA2}
~ \includegraphics[width=4.1cm]{Fig_d1VaB1_LDOS_c05pc_VaB2}

\vspace{.1cm}

\caption{ \label{Fig_DOS_d1A1_B1}
Electronic structure of BLG with TB1 (nearest neighbor hopping):
In BLG with A$_2$ vacant atoms:
(a.1) total DOS, $n'$  (dashed line is TDOS without vacancy),
(a.2) average local DOS $n_i'$ on $i=$ A$_1$, B$_1$, A$_2$, B$_2$ atoms with $c=0.5$\% (dashed line and dot line are LDOS on A and B atom without vacancy).
In BLG with B$_2$ vacant atoms:
(b.1) total DOS $n'$ (dashed line is TDOS without vacancy),
(b.2) average local DOS $n_i'$ on $i=$ A$_1$, B$_1$, A$_2$, B$_2$ atoms $c=0.5$\%
(dashed line and dot line are LDOS on A and B atom without vacancy),
$c$ is the concentration of vacancies with respect to the total number of atom in BLG.
The spectrum is symmetric with respect to Dirac energy $E_D=0$.
DOS are calculated from (\ref{eq_nepsilon}) with $\epsilon = 5$\,meV.
}

\vskip 0.5cm

\includegraphics[width=4.1cm]{Fig_d1VaA1_tDOS_mLor_v2}
~ \includegraphics[width=4.1cm]{Fig_d1VaB1_tDOS_mLor_v2}~

\vspace{.1cm}
\includegraphics[width=4.1cm]{Fig_d1VaA1_LDOS_c05pc_mLor_VaA2}
~ \includegraphics[width=4.1cm]{Fig_d1VaB1_LDOS_c05pc_mLor_VaB2}

\caption{ \label{Fig_DOS_d1A1B1_mLor}
Same DOS and LDOS than figure \ref{Fig_DOS_d1A1_B1}, but without drawing the midgap states at $E=0$.
$n$ (without midgap) is computed from $n'$ (with midgap states) by equations (\ref{Eq_DOS_avec_sans_Lor}) and (\ref{Eq_DOS_avec_sans_Lori}).
}
\end{center}
\end{figure}

\section*{2. Midgap states in case of first neighbor hopping model (TB1) with vacancies on a sublattice only}
\label{subLorentzienne}

\begin{figure}
\begin{center}
\includegraphics[width=6cm]{Fig_LaA1_05pc_tDOS_Lor}

\vspace{.1cm}
\includegraphics[width=6cm]{Fig_LaA1_05pc_DOSB1_Lor_A2}

\caption{Electronic density of states in BLG  with A$_2$ vacant atoms ($c=0.5$\%):
(a) Calculated total DOS $n'(E)$,  $n'(E)=n(E) + x L(E)$, $x=0.01$;
(b) Calculated average local DOS on B$_2$ atoms $n_{B_2}'(E)$, $n_{B_2}'(E)=n_{B_2}(E) + x_{2} L(E)$, $x_2 = 0.04016$,
where $L(E)$ is the Lorentzian of the midgap states at $E=0$ that are located only on B$_2$ sublattice, and
$n(E)$ and $n_{B_2}(E)$ are, respectively, the exact total DOS and the exact average local DOS on B$_2$ sublattice at all energies except at $E=0$.
\label{Fig_DOS_LaA1_avec_sans_Lor}
}
\end{center}
\end{figure}

\begin{figure}
\begin{center}
\includegraphics[width=6cm]{Fig_LaB1_05pc_tDOS_Lor}

\vspace{.1cm}
\includegraphics[width=6cm]{Fig_LaB1_05pc_DOSA1_Lor_LaB2}

\vspace{.1cm}
\includegraphics[width=6cm]{Fig_LaB1_05pc_DOSB2_Lor_LaB2}

\caption{Electronic density of states in BLG  with B$_2$ vacant atoms ($c=0.5$\%):
(a) Calculated total DOS $n'(E)$,  $n'(E)=n(E) + x L(E)$, with $x=0.010099$;
(b) Calculated average local DOS on A$_2$ atoms $n_{A_2}'(E)$, $n_{A_2}'(E)=n_{A_2}(E) + x_2 L(E)$, with $x_2 = 0.032573$;
(c) Calculated average local DOS on B$_1$ atoms $n_{B_1}'(E)$, $n_{B_1}'(E)=n_{B_1}(E) + x_1 L(E)$, with $x_1 = 0.0070745$.
$x_1 L(E)$ and $x_2 L(E)$ are the Lorentzian of the midgap states at $E=0$ located on B$_1$ sublattice and A$_2$ sublattice, respectively.
$n(E)$ and $n_{i}(E)$ are, respectively, the exact total DOS and the exact average local DOS on $i$ sublattice at all energies except at $E=0$.
\label{Fig_DOS_LaB1_avec_sans_Lor}
}
\end{center}
\end{figure}

The total density of states (total DOS) $n'$ is computed by recursion (Lanczos algorithm) \cite{methodeRecursion} in real-space on sample containing $N$ carbon atoms, $N$ is up to a few $10^{7}$, with periodic boundary conditions.
Considering a random phase states $\varphi_0$,  \cite{Roche97}
\begin{equation}
 \left | \varphi_0  \right \rangle = \frac{1}{\sqrt{N}} \sum_{m=1}^{N} {\rm e}^{i 2 \pi \theta_m}   \left | \Phi_m \right \rangle,
\end{equation}
where  $\left | \Phi_m  \right \rangle$ the $p_z$ orbital of atom $m$
and $\theta_m$ is a random number between 0 and 1,
the total DOS $n'$ is
\begin{equation}
n'(E) =  \lim_{\epsilon \to 0^+} n'(E,\epsilon),
\end{equation}
with
\begin{equation}
n'(E,\epsilon) = - \frac{1}{\pi} {\rm Im} \left \langle \varphi_0 \right | \frac{1}{E + i \epsilon - \hat{H}}  \left | \varphi_0  \right \rangle.
\label{eq_nepsilon}
\end{equation}
The DOS $n'$ at energy $E$ is thus evaluated numerically from a continuous fraction expansion of the Green function, $G(z) = 1 / (z-\hat{H})$, with $z = E + i \epsilon$ and a finite small $\epsilon$ value \cite{methodeRecursion}.
Therefore, the computed DOS $n'$ is the real DOS convoluted with the Lorentzian function,
\begin{equation}
L(E,\epsilon) = \frac{\epsilon}{\pi} \frac{1}{E^2 + \epsilon^2},
\label{eq_Lorent}
\end{equation}
of half width $2 \epsilon$.
Roughly speaking, $\epsilon$ is a kind of energy precision of the calculation. As $\epsilon$ is small, $N$ should be large.
DOSs presented in this paper are computed with $\epsilon = 5$\,meV.

Average local DOSs, $n_i'$ on a $i$ sublattice, $i=$ A$_1$, B$_1$, A$_2$, B$_2$ are obtained using the same numerical method with a
random phase $\varphi_{0i}$ expands on the $p_z$ orbitals $ \Phi_{m_i}$  of the $i$ sublattice,
\begin{equation}
 \left | \varphi_{0i}  \right \rangle = \frac{1}{\sqrt{N_i}} \sum_{m_i=1}^{N_i} {\rm e}^{i 2 \pi \theta_{m_i}}   \left | \Phi_{m_i} \right \rangle ,
\end{equation}
where $m_i$ is the index of atoms of the $i$ sublattice that contains $N_i$ atoms.
Figure \ref{Fig_DOS_d1A1_B1} shows total DOS and average local DOSs $n'$, calculated with TB1,
for BLG with vacancies on A$_2$ and B$_2$ sublattice respectively.

As explained in the paper, with TB1 model and a $\alpha$-$\beta$ bipartite lattice, vacancies in the $\alpha$ sublattice involve midgap states, at energy $E_{MG}=0$, that are located on $\beta$ sublattice.
Because of the convolution with the Lorentzian (\ref{eq_Lorent}), the calculated total DOS $n'$ and average local DOS $n_i'$, $i=$ A$_1$, B$_1$, A$_2$, B$_2$ can be written as
\begin{equation}
n'(E,\epsilon) = n(E,\epsilon) + x L(E,\epsilon),
\label{Eq_DOS_avec_sans_Lor}
\end{equation}
and
\begin{equation}
n_i'(E,\epsilon) = n_i(E,\epsilon) + x_i L(E,\epsilon),
\label{Eq_DOS_avec_sans_Lori}
\end{equation}
where $x$ ($x_i$) is proportional of the concentration $c$ of vacant atoms, $x L$ ($x_i L$) is the calculated DOS due to midgap states,
and $n$ ($n_i$) is the DOS (LDOS) without the midgap states.
$n'(E)$ ($n_i'(E)$) is computed by recursion method from  equation (\ref{eq_nepsilon}) with $\epsilon = 5$\,meV,
and $n(E,\epsilon)$ ($n_i(E,\epsilon)$)
is computed from  $n'(E,\epsilon)$ ($n_i'(E,\epsilon)$) by equation ({\ref{Eq_DOS_avec_sans_Lor}) (equation ({\ref{Eq_DOS_avec_sans_Lori})).
The total DOSs $n$, shown in the main paper figures
2(1.a)
and
2(1.b)
(see also figures \ref{Fig_DOS_d1A1B1_mLor}(a.1) and \ref{Fig_DOS_d1A1B1_mLor}(b.1)),
correspond respectively to total DOSs $n'$ shown figures \ref{Fig_DOS_d1A1_B1}(a.1) and \ref{Fig_DOS_d1A1_B1}(b.1).
Showing $n$ instead of $n'$
allows to discuss more explicitly the DOS around $E_{MG} = 0$
and to show the presence of quasi-gap. This quasi-gap is hidden by the midgap state Lorentzian in DOS $n_t'$.
Figures \ref{Fig_DOS_LaA1_avec_sans_Lor} and  \ref{Fig_DOS_LaB1_avec_sans_Lor} show several examples of the three terms of equations (\ref{Eq_DOS_avec_sans_Lor})-(\ref{Eq_DOS_avec_sans_Lori}).
With A$_2$ vacant atoms (figure \ref{Fig_DOS_d1A1_B1}(a.2) and figure \ref{Fig_DOS_LaA1_avec_sans_Lor}), the midgap states
($i.e.$ term $L(E)$ in equations (\ref{Eq_DOS_avec_sans_Lor}-\ref{Eq_DOS_avec_sans_Lori}))
are located on B$_2$ sublattice.
With B$_2$ vacant atoms (figure \ref{Fig_DOS_d1A1_B1}(b.2) and figure \ref{Fig_DOS_LaB1_avec_sans_Lor}),
the midgap states are located both on A$_2$ sublattice and B$_1$ sublattice.

\section*{3. Eigenstates of a square bipartite lattice with vacancies in a sublattice}

\begin{figure}
\begin{center}

\includegraphics[width=7cm]{Fig_carre4pc_DOS}

\includegraphics[width=7cm]{Fig_carre4pc_DOSmLor}

\includegraphics[width=7cm]{Fig_carreLa1_dos-1_Nr3mEps2meV}

\includegraphics[width=7cm]{Fig_carreLa1_dos-1_Nr5mEps02meV.pdf}

\caption{ \label{Fig_DOS_bipartite_carre}
Bipartite square lattice with two atoms, A and B, per unit cell, and vacancies in the A (or B) sublattice:
(a) Total DOS, $n'$, and average local DOS, $n_A' = n_A$ ($n_B'$), on A sublattice (B sublattice), for $c=4\%$ of vacant A atoms  and $\epsilon = 2$\,meV
[Inset: total DOS $n'$].
(b) Total DOS $n$ and average local DOS $n_A$ ($n_B$) on A sublattice (B sublattice), for $c=4\%$ of vacant A atoms  and $\epsilon = 2$\,meV
[Inset: total DOS $n$].
(c) and (d) Total DOS $n$ for various concentrations $c$ of vacant A atom. $c$ is the concentration of vacancies with respect to the total number of atoms in the lattice: (c) with $\epsilon = 2$\,meV and (d) $\epsilon = 0.2$\,meV.
}
\end{center}
\end{figure}

In this section, we consider a simple square lattice containing two atoms in a unit cell: atom A in position $(0,0)$ and atom B in position $(1/2, 1/2)$.
Only $s$ orbitals are taken into account and the Hamiltonian includes only nearest-neighbor hopping between orbitals:
\begin{equation}
\hat{H} = \sum_{\langle i,j \rangle} t_{ij} \left( c_i^{\dag}c_j + c_j^{\dag}c_i \right),
\label{Eq_hamiltonian_SupMat2}
\end{equation}
where $c_i^{\dag}$ and $c_i$ create and annihilate respectively an electron on the $s$ orbital located at $\vec r_i$,
$\langle i,j\rangle$ is  the sum on index $i$ and $j$ with $i\ne j$,
and  $t_{ij}$ is the hopping matrix element
between two orbitals located at $\vec r_i$ and $\vec r_j$.
Each atom A is coupled with only B atoms and reciprocally.
This lattice is thus a bipartite lattice with two equivalent sub-parts  $\alpha$ and $\beta$  corresponding respectively to atoms A and atoms B.

We consider  vacancies (missing atoms) distributed randomly in the A sublattice.
As explained in previous section (section 2), we calculated DOS, $n_i'$, $i = t$ (total), A, B
(figure \ref{Fig_DOS_bipartite_carre}(a))
and the DOS $n_i$, $n_i(E) = n_i'(E) - x_i L(E)$,
(figure  \ref{Fig_DOS_bipartite_carre}(b)).
The Lorentzian of the midgap states at $E=0$ is clearly seen on total DOS, $n'$,  and average local DOS, $n_B'$, on the B sublattice.
As expected from the bipartite analysis explained in the paper, vacancies in a sublattice result in a gap between  $-E_{min}$ and $E_{min}$.
The energy gap
$2E_{min}$ increases as the concentration $c$ of vacancies increases
(figures \ref{Fig_DOS_bipartite_carre}(c,d)).

These calculations are performed by recursion in a supercell (section 2) containing $N=2 \times 2400^2 = 23.04 \times 10^6$ atoms.
Figures \ref{Fig_DOS_bipartite_carre}(a,b,c) presents DOS calculated with $\epsilon= 2$\,meV. In this case, the convolution with the Lorentzian of width $2\epsilon$ hides the gap when the concentration of vacancies is small. To check the presence of real gap, we show DOS calculated with $\epsilon= 0.2$\,meV in figure \ref{Fig_DOS_bipartite_carre}(d). In this case, gap in clearly seen at all calculated vacancy concentrations, but unphysical oscillations appeared in DOSs.
Those oscillations  are due to numerical artifact related to the termination of the
continuous fraction expansion of the Green function (equation  (\ref{eq_nepsilon})) in presence of a gap \cite{methodeRecursion}.

\section*{4. Numerical method for conductivity}

\subsection*{4.1. Kubo-Greenwood scheme}

In Kubo-Greenwood formula for transport properties,
the quantum diffusion $D$, is computed by using the polynomial expansion of the average square spreading, $\Delta X^{2}$, for charge carriers.
This method, developped by Mayou, Khanna, Roche and Triozon \cite{Mayou88,Mayou95,Roche97,Roche99,Triozon02},
allows very efficient numerical calculations by recursion in real-space that taken into account all quantum effects.
It has been used to studies quantum transport in disordered graphene
\cite{Lherbier08,Lherbier11,Leconte11,Leconte11b,Roche12,Roche13,Trambly13}
and chemically doped graphene \cite{Lherbier08b,Leconte10}.
Static defects are included directly in the structural modelisation of the system and they are randomly distributed on a supercell containing up to $10^7$ Carbon atoms.
This corresponds to typical sizes of about one micrometer square which allows to study systems with inelastic mean-free length of the order of few hundreds nanometers.
Inelastic scattering is computed \cite{Trambly13} within the
Relaxation Time Approximation. An inelastic scattering time $\tau_i$ beyond which the propagation becomes diffusive due to the destruction of coherence by inelastic process. One finally get the Einstein conductivity  formula (at $0$\,K), \cite{Trambly13}
\begin{equation}
\sigma(E_F,\tau_i) = e^2 n(E_F) D(E_F,\tau_i),
\label{eq_einstein}
\end{equation}
where $E_F$ is the Fermi level,
$D(E,\tau_i)$ is the diffusivity (diffusion coefficient at energy $E$ and inelastic scattering time $\tau_i$),
\begin{equation}
D(E,\tau_i) = \frac{L_i^2(E,\tau_i)}{2 \tau_i},
\end{equation}
$n(E)$ is the density of states (DOS) and $L_i(E,\tau_i)$ is the inelastic mean-free path. $L_i(E,\tau_i)$ is the typical distance of propagation during the time interval $\tau_i$ for electrons at energy $E$,
\begin{equation}
L_{i}^{2}(E,\tau_{i})=\frac{1}{\tau_{i}} \int_0^\infty \! \Delta X^{2}(E,t)\,{\rm e}^{-t/\tau_{i}}  .
\end{equation}
Without static defects (static disorder) the $L_i$ and $D$ goes to infinity when $\tau_i$ diverges.
With statics defects, at every energy $E$, $\sigma(\tau_i)$ reaches a maximum value,
\begin{equation}
\sigma_m(E_F,\tau_i) = e^2 n(E_F) \, {\rm Max}_{\tau_i} \left \{ D(E_F,\tau_i) \right \},
\label{eq_einstein_SigM}
\end{equation}
called
microscopic conductivity. $\sigma_m$ corresponds to the usual semi-classical approximation (semi-classical conductivity).
This conductivity is typically the conductivity at room temperature, when inelastic scattering $\tau_i$ (inelastic mean free path $L_i$) is closed to elastic scattering $\tau_e$ (elastic mean free path $L_e$), $\tau_e(E) = L_e(E) / v(E)$ and $L_e(E) = D_m(E) / 2 v(E)$, where $D_m(E)$ is the maximum value of $D(\tau_i)$ at energy $E$ and $v(E)$ the velocity at very small times (slope of $\Delta X(t)$).

For larger $\tau_i$ and $L_i$, $\tau_e \ll \tau_i$ and $L_e \ll L_i$, quantum interferences may result in a diffusive state,
$D(\tau_i) \simeq D_m$, or a sub-diffusive state where $D$ decreases when $\tau_i$ and $L_i$ increase.
For very large $L_i$, $L_i$ closed to localization length $\xi$, the conductivity goes to zero.
These two last regimes ($L_e \ll L_i$, and  $L_i \simeq \xi$), which correspond to the low temperature regime,  are not discussed in the main paper.

\begin{figure}
\begin{center}

\includegraphics[width=4.2cm]{Fig_d1VaA1_SigM}
~ \includegraphics[width=4.1cm]{Fig_d1VaB1_SigM}

\vspace{.1cm}
\includegraphics[width=4.1cm]{Fig_d1VaA1_SigM_mLorDOS}
~ \includegraphics[width=4.1cm]{Fig_d1VaB1_SigM_mLorDOS}

\caption{ \label{Fig_DOS_Sig_d1A1B1_mLorDOS}
Microscopic conductivity  $\sigma_m(E)$ computed from TB1 in BLG:
for A$_2$ vacant atoms [(a.1) (a.2)],
and for B$_2$ vacant atoms [(b.1) (b.2)].
$\sigma_m(E)$ is computed from equation (\ref{eq_einstein})
where (a.1) (b.1) the total DOS $n(E)$ includes Lorentzian due to midgap states at $E=0$,
and (a.2) (b.2) $n(E)$ excludes the Lorentzian due to midgap states at $E=0$.
$c$ is the concentration of vacancies with respect to the total number of atom in BLG.
Spectrum is symmetric with respect to Dirac energy $E_D=0$.
}
\end{center}
\end{figure}

\subsection*
4.2. Midgap states in case of first neighbor hopping model (TB1) with vacancies on a sublattice only}

As discussed section 2, with first neighbor hopping model (TB1) and vacancies in only one sublattice, midgap states are found at the energy $E_D = 0$. These states are not coupled to each other by $H$; thus they do not contributed to the DOS and the conduction properties at $E \ne 0$.
For this reason, the conductivity presented in the main paper is computed numerically by equation (\ref{eq_einstein_SigM}) using the total DOS $n(E)$ that does not included the Lorentzian due to midgap states at $E = 0$ (section 2 of this Supplementary Material).
Microscopic conductivity computed with and without this Lorentzian contribution to the DOS is shown figure \ref{Fig_DOS_Sig_d1A1B1_mLorDOS}.

Therefore our study does not deal with conduction by midgap states at $E \ne 0$ in the case of first neighbor hopping model (TB1).
Nevertheless the results with the more realistic Hamiltonian TB2, that includes hopping beyond first neighbor, show that midgap states in TB1 model are very specific to TB1 model and are not realistic in real bilayer graphene, as it has been found for the monolayer graphene \cite{Trambly14}.

\section*{References}

redpajama_set_name: RedPajamaArXiv


text:
O Campeonato do Mundo de Tosquia (ou Tosa) de Ovelhas é uma competição de tosa de ovelhas que acontece a cada 2 anos.

O objetivo do esporte é simples: Com uma tesoura própria, cada competidor deve tosquiar (ou tosar) sua ovelha no menor tempo possível. Os maiores especialistas da área são os neozelandeses, que inclusive detém o recorde mundial (20 segundos).

Em 2012 aconteceu o 50º Campeonato, e foi sediado no Molyneux Park Stadium, na cidade de Alexandra.

Ligações externas
terratv.terra.com.br
esporte.uol.com.br
wairarapanz.com
rwas.co.uk

Tecidos têxteis

redpajama_set_name: RedPajamaWikipedia


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text:
Mount St. Bride är ett berg i Kanada.   Det ligger i provinsen Alberta, i den centrala delen av landet,  km väster om huvudstaden Ottawa. Toppen på Mount St. Bride är  meter över havet.

Terrängen runt Mount St. Bride är kuperad västerut, men österut är den bergig. Den högsta punkten i närheten är  meter över havet,  km norr om Mount St. Bride. Trakten runt Mount St. Bride är nära nog obefolkad, med mindre än två invånare per kvadratkilometer.. Närmaste större samhälle är Lake Louise,  km sydväst om Mount St. Bride.

Trakten runt Mount St. Bride består i huvudsak av gräsmarker.  Trakten ingår i den boreala klimatzonen. Årsmedeltemperaturen i trakten är  °C. Den varmaste månaden är juli, då medeltemperaturen är  °C, och den kallaste är december, med  °C.

Kommentarer

Källor

Berg i Alberta
Berg i Kanada 2000 meter över havet eller högre


Never miss a chance to throw in a 'climate warming' reference. While you're at it why not throw in Trump Russian Collusion? My point is to leave the politics out of scientific discussions.
It appears to me that you are the one who can't take politics out of scientific discussions.
"The Sun reached a peak in activity during 2014. It turned out to be the weakest maximum in solar activity since 1906. Solar activity has since been declining and will soon bottom out. There are indications that this upcoming solar minimum could be particularly deep". We are in a hyperdementional gyroscopic sphere of shared energy where if this than opposed is given. This phenomenon has absolutely nothing to due with Hawaiian eruption.
We are all about to find out just how insignificant man, and his activities are, in the face of the sun itself.
You haven't met the scientists at cern and fermilabs if that's your opinion.
Do you know what a particle accelerator is?
Pull your cranium out of your posterior and actually examine the effects of using that device. Do you REALLY know what an accelerator is? Go Learn!
It's important to point out the limited nature of the so-called "Little Ice Age" attributed to the Maunder-Minimum. As noted in the article, the effects seem limited primarily to Europe, but did not produce a substantial cooling planet wide. Certainly nothing approaching the mildest of the ice ages during human prehistory. Yet some are quick to claim climate change due to human activity will be erased, or even replaced by a mini ice age, once the next episode of minimum solar activity occurs. The evidence from world history strongly disputes that. Our sun is without doubt the single greatest force impacting the global climate, but it is a remarkably stable star — which is why we're all here to have this conversation. Nothing in recorded history suggests solar energy output will change drastically enough in the foreseeable future to overwhelm the impact humanity's massive input of greenhouse gases is having on our world.
No ,the effects of the LIA were not limited to Europe . They were global in extent ,just most documented in Europe .
Global ocean studies show ~ 1C cooling 1300 1650 .. both hemispheres.
See Oceans 2k 2015 ,Rosenthal et al 2013 .
The undetermined but assumed human impact on GAST is about to get a whole new review . .
The actual effects on land are much less clear, and Rosenthal 's overall work supports the fact that the oceans are warming more quickly now than in the past, driven by AGW.
Well , the effects on land are actually quite clear . Warmer sea surfaces in particular cause warmer and moister conditions on land ,without exception . See effects of ENSO . AMO and PDO phases.
The point was both studies agree on global MWP and LIA , both studies agree on temps at 1100 AD and 1700 AD .
The rate of warming for the top 2,000 ms of the oceans is ~ 0.2C century . several centuries till MWP temps are matched .
That's a lot of acronyms, and still no actual proof that current warming is natural, or that the vast majority of scientists who blame it on carbon emissions are incorrect.
I see you want to change the subject from the MWP and the LIA to current warming ? I don't blame you !
The claim that current warming is not natural is the claim that requires "proof" .
In science , the null is assumed correct absent conclusive and indisputable evidence the null hypothesis is wrong or invalid.
In the instant case ,no such evidence exists .,regardless of the number of scientists that support the CO2 explanation for post 1950 temps .
Good thing there's actually a ton of proof in the form of research and observation, which is why the scientific consensus is that it isn't natural. So your contrarian position does require proof, and not just your strident assertion.
If you knew anything about science ,you would know the word "proof" does not apply .
"Proof" is used in math and logic . and "consensus" does not confer or imply validity to a theory or hypothesis . .
I suggest you look into the Continental Drift controversy ,the 99% consensus of last century was that the continents were "fixed" , and the "ton of proof" explained the matching coasts , strata and fossils as a "co incidence" .
An error that lasted over 50 years ,until about 1970 .
Pleased you have dropped the no global MWP or LIA claims .. some progress ,but ,you have far to go ..
It is interesting that the very kinds of technology that finally provided hard evidence and confirmation for Wegener's idea and posthumous vindication have also enabled modern climate science to know things about the earth's climate to a high degree of confidence–things that you and your fellow climate science dismissives like to pretend don't exist.
Of course, comparing the state of "consensus" in paleo-geology of over a century ago, where there were only a tiny handful of researchers, to modern climate science today, with thousands of researchers availed of massive amounts of satellite data and field data gathered from the most remote parts of the earth, is the height of apples-to-oranges absurdity.
And your leap from a correct statement about "proof" to an insinuation that "consensus" is a meaningless term is worthy of your most wildly dishonest prestidigitations.
So, Richard Muller's research was wrong when he found the strongest correlation to modern warming in anthropogenic CO2? It's curious how you view his non-peer-reviewed and baldly incorrect opinions about Mann as definitive but dismiss his actual research.
Claiming that "no such evidence exists" for the overwhelming consensus view of active research scientists is the height of ignorance.
–except where warmer temperatures intensify drought and reduce availability of water, as has happened in several hot spots around the globe.
Your little "without exception" is where you fall apart, dimwit.
There's actually good research showing a very consistent temperature signal mapping against past solar minimums — not just the Maunder Minimum. We're seeing more and more data suggesting that we're heading into a new minimum but I don't think anyone at this point knows how serious a drop in solar forcing this will produce. The good news is that a lot of people are starting to look at this issue more seriously and searching for ways to project more accurately expected changes in solar forcing.
You may want to purchase some property near Presidio, Texas, which is often the hottest reported city in North America. For some strange reason it is also the longest continuously inhabited area in North America.


When you hire a marketing agency to help your business, one of the first things they want to know is "who is your target market?" For Clayton Homes, one of their biggest markets has been and always will be the affordable home crowd.
These are the good hard working people that mostly hold blue collar jobs, have strong family values, go to church and like to have fun. They have been portrayed through families like Honey Boo Boo's and Duck Dynasty. In other words, they are the people that form the backbone of our nation.
Well, Clayton Homes is no stranger to trying to put this target market into their brands of homes but when they signed Si from Duck Dynasty to be their spokesperson, they immediately acquired a built-in audience of millions of fans. Click Here to read about Si choosing a Clayton Home.
Is it working? I have a feeling that is a close guarded secret within the Clayton Homes boardroom but from all the indications I've seen, it has been very successful.
Here is a video of just one small part of Clayton's efforts to win over the affordable housing crowd.
Clayton is preaching to the choir. The industry needs to market to the other 85% of the home buying public and find new customers! Not continue to be satisfied with the same demographic year after year.


Time to pray photo & image | architecture, sacred buildings, mosque images at photo community Time to pray Photo & image by .N.i.c.o.l.a.s. ᐅ View and rate this photo free at fotocommunity.de. Discover more images here.


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Here's hoping you are enjoying time with your family and friends during the Thanksgiving holiday!
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Description: The church in Suurhusen is reminiscent of the old fortress churches of old. Originally the church was 32 metres long and 9.35 metres wide. The church tilts at an angle of 5.19 degrees compared to just 3.97 degrees for the Pisa tower. In 1450 the church was shortened by about a quarter and the tower was built in the space. This tower is considered today to be the most leaning tower in the world and is known as the Leaning Tower of Suurhusen.
According to local historian Tjabbo van Lessen, the church was built in marshy land in 1450 on foundations of oak tree trunks which were preserved by the water in the ground. When the land was drained in the 19th century, the wood rotted, causing the tower to tilt. The steeple was closed to the public in 1975 for safety reasons, but re-opened 10 years later after being made safe.