text:
The Nice Guys: Gosling, Crowe & Seventies Porn in Odd-Couple 70s Detective Comedy
Russell CroweRyan Gosling
Action & AdventureComedy
In 1 Cinema
Marija Loncarevic
Snappy dialogue, deadpan humour and a refreshingly pleasing no-nonsense mindset are just some of the components that make Shane Black's latest cinematic effort, The Nice Guys, a hilarious retro buddy-action-comedy which, although not always smooth in its delivery, manages to offer plenty of excitement and genuine moments of hilarity.
Set against the somewhat sleazy backdrop of 1977 Los Angeles, the story follows unlucky-in-pretty-much-everything private investigator and single father, Holland March (Gosling), who has been hired to solve the mystery around the death of Misty Mountains (Tello); a famous adult film star who was allegedly spotted soon after the car accident that supposedly killed her.
Without offering it too much thought, Holland takes on the case and the trail soon brings him to his first – and only – lead; a young woman named Amelia (Qualley) who was apparently seen with Misty right before her 'death'. However, before Holland gets a chance to investigate further, he is stopped by Jackson Healy (Crowe); a cold and brutal muscle-for-hire who also happens to be looking for Amelia after being recruited by her politically influential mother, Judith (Basinger).
Coming to realise, that they will require each other's set of skills to get the job done, the pair soon find themselves deep inside the adult film underworld, where uncovering the truth is not as easy as they thought.
It takes a little while to get The Nice Guys on a an even road with the movie's opening minutes a bit on the messy side with Black struggling to strike the right kind of balance and tone to set the story that is to come. However, things soon even out when the two investigators – hands-down one of the best onscreen pairings we've seen in a while – are united, with their almost-palpable chemistry and comic energy pushing the plot forward.
Gosling and Crowe are the heart of the story with the merciless but somehow loveable Healy working in perfect comedic harmony with the fast-talking and at-times weepy Holland. The 70's backdrop is crafted with a great amount of detail, offering a genuinely retro feel – which serves to be almost a supporting character in the story – and a throwback to a time where sex, drugs and rock and roll were the order of the day.
Funny and occasionally pleasingly absurd, there are no nice guys in The Nice Guys, just a couple of endearing losers who will have you in stitches.
Like This? Try
Kiss Kiss Bang Bang (2005), Lethal Weapon (1987), Starsky & Hutch (2004)
360 Tip
First film directed by Shane Black to not star Robert Downey Jr.
Your Guide to the Differences Between Credit and Debit Cards
city life credit cards +3
Cairo's Eye is set to Open Next Year
A-Plus Firm Ain Cairo +6
COVID-19 Vaccine Locations in Egypt Finally Announced
city life COVID-19 +3
Bridgerton: A Period Drama Like Never Before Featuring 104 Dresses
Bridgerton Fashion +2


Located at the south end of the island, on the Bukit peninsula, the Uluwatu area is famous for it's variety of surf spots. Uluwatu is different from other parts of the island as it's situated on the cliff tops with beach access found through small staircases cut into the rock. This allows for some great sunset views and a much more local vibe.
DO catch some waves/sun and relax at the various beaches. Most beaches are a 15-20 minute scooter ride away from each other, and beach access costs approx. $0.15 to $0.55 USD (pay at the entrance or gates near parking areas). Below is a quick overview of our experience at the different beaches.
Bingin Beach - One of the smaller, more quiet and quaint beaches is Bingin. It often feels like a slice of paradise nestled among a cliff side of lovely rental homes and a few restaurants. The waves here tend to be more calm - allowing for surfers and swimmers of all ages/experience. To access the beach you will need to walk down a fairly narrow and steep series of cobblestone steps.
Padang Padang Beach - This is one of the more well known beaches in the area. We found it beautiful but rather small with quite a lot of tourists.
Uluwatu Beach - One of the most famous beaches in Bali for surfers. It's powerful waves and reef bottom make it a more advanced surf spot. If you're interested in lounging on the beach to watch, know that you'll have to sneak through a very small hole in the cliff side or wait until low tide to walk out. We enjoyed watching the surfers from the cliff top at Single Fin.
Balangan Beach - This beach was larger than Bingin or Padang Padang and offered beautiful white sand with great views of the surrounding cliffs. There are also many traditional restaurants and surf rental shops lining the beach. Balangan seemed to be be one of the better beaches for beginner surfers looking to catch some waves.
EAT at Nalu Bowls for the best smoothie bowls we've had yet in Bali!
We'd also recommend Buddha Soul for fresh, flavorful vegan meals. You will not be disappointed by the sticky black rice with a latte for breakfast or the vegetable pesto rice bowl for lunch.
Try Kelly's Warung at Bingin Beach for a variety of wraps, smoothies, and delicious traditional options.
If you're willing to try very traditional food we enjoyed Warung Heboh. You pay per scoop of food and dish yourself. Huge plates of food typically cost us approx. $2 USD and everything we tried was delicious.
DRINK and enjoy the music at Single Fin during sunset. (Yes, drinking beer at the beach during sunset is one of our favorite things to do!) We recommend getting a reservation online otherwise go early (around 4 PM) to get a seat. There's a lengthy dinner menu here also, with options ranging from pizza and burgers to steak.
STAY somewhere central to all beaches or splurge for a place with a view. We stayed near Padang Padang beach which ended up being very central and convenient. We'd love to hear more about the hotel and infinity pool overlooking the ocean at Blue Point (right next to Single Fin). Sunsets from this pool look dreamy!
CRUISE anywhere by scooter. Since most destinations and shops are spread out around Uluwatu, we highly recommend renting one for the entire time you're here. Daily scooter rentals average approx. $3-5 USD - it's cheaper if you do a weekly rental. You can find gas at Petrol stands all throughout town. Two glass bottles of gas (usually Absolut Vodka bottles) will fill your tank for approx. $1 USD.
KNOW although typically somewhat easy to find, Uber is frowned upon in the Kuta and Uluwatu areas of Bali. You'll see signs with a big red X through the logo and locals will tell you not to use them. We had a great experience with our Uber driver but were later told Uber isn't allowed here. Uncertain of the reasoning here.


Malformed Fingers are outlined in the amazing pictographs at Shaman's Gallery in the Grand Canyon's North Rim.
Roundhead Blank Face: I'm tempted to call these guys pinheads but pins did not exist 3,000 years ago when this was painted on the rock wall.
Runyon Canyon Sunrise over the city of Los Angeles. I didn't see any stars but enjoyed seeing sunrise over the city and the ocean in the distance.
Fog over Saint Louis hide the arch in a misty white color.
Exit Arrow pointing the way out of the Herzog and de Meuron parking structure in South Beach, Miami.
Shark Valley Observation Tower can be found at the end of a long 7-mile ride or walk. The tower overlooks the swamp, alligators, birds and flat land of the everglades.
London Architecture with two contrasting buildings.
Stonehenge and Raven in black and white. The brooding low clouds settled over the stone circle.
Stonehenge Panoramic Stone Circle taken from a distance on an absolately beautiful day.
Millstones at Stannage Edge sit for hundreds of years. The green valley watches.
Ladybower Spillway on the Ladybower Reservoir in the Peaks District. This eye-catching dam and spillway hypnotizes with intermingling circles and depth.
Winnat's Pass Road is narrow with sharp turns and deep green grass surrounding every side. Drive slowly and enjoy the view.
Fountains Abbey Hallway with arches, columns and light in black and white.
June 2016: Prebend's Bridge Morning, a silent and peaceful spot along the Wear River. This Durham Bridge is most beautifully seen from one of the lovely walks along the river. Green trees hang over each bank. The stone bridge has three wonderful arches.
Hadrian's Wall Zig Zag along the course of the Steel Rigg area and Housesteads Roman fort. This is the most beautiful portion of the wall.
Red Brick of Fort Zachary Taylor Inside the shadows and light stretch across long empty corridors. The feeling of being here is remarkable.
Jefferson Monument: the bases of round columns.
Grafton Schoolhouse, near Zion is a stately building in a ghost town.


text:
Madhusmita Somnath Behera (born 4 October 1990 at Cuttack, Orissa) is an Indian cricketer. She is a right-handed batsman and bowls right-arm off-break. She plays for Odisha and East Zone. She has played 8 First-class, 71 List A and 43 Women's Twenty20.

References

1990 births
Living people
People from Cuttack
Cricketers from Odisha
Sportswomen from Odisha
Odisha women cricketers
East Zone women cricketers
Indian women cricketers

redpajama_set_name: RedPajamaWikipedia


TriCEM is hosting a breakfast featuring Dr. Adrian Jaeggi. He will be giving a lecture titled Testing the SES/health gradient and inequality and health associations among the Tsimane of Bolivia: An evolutionary medicine approach.
In addition, Dr. Adrian Jaeggi of Emory University will be giving a seminar in Evolutionary Anthropology titled Comparative behavioral ecology: Recent studies on bonobo and human cooperation.


text:
package wsa.submission.fromwsdl.crinterop.s11.server;

import java.util.Calendar;
import java.io.IOException;

import jakarta.xml.ws.WebServiceProvider;
import jakarta.xml.ws.ServiceMode;
import jakarta.xml.ws.Service;
import jakarta.xml.ws.Provider;
import jakarta.xml.soap.SOAPMessage;
import jakarta.xml.soap.SOAPException;

/**
 * @author Arun Gupta
 */
@WebServiceProvider
@ServiceMode(value = Service.Mode.MESSAGE)
public class NonAnonymousProvider implements Provider<SOAPMessage> {
    public SOAPMessage invoke(SOAPMessage request) {
        System.out.printf("====%s[start:%tc]====\n", getClass().getName(), Calendar.getInstance());
        try {
            request.writeTo(System.out);
        } catch (SOAPException e) {
            e.printStackTrace();
        } catch (IOException e) {
            e.printStackTrace();
        }
        System.out.printf("====%s[end:%tc]====\n", getClass().getName(), Calendar.getInstance());
        return null;
    }
}

redpajama_set_name: RedPajamaGithub


Only Milo is a gold medal winner!
Only Milo, by Barry Smith, won the Gold Medal in Popular Fiction in the 2010 Independent Publisher Book Awards. In this darkly funny spoof of the publishing world, Milo is tired of being underestimated, and his path to notoriety is fraught with deception, forgery, theft, and murder.
The Independent Publisher Book Awards ("IPPY") strives to recognize the best independent authors and publishers with their annual award program. For a full list of award winners you can visit their site.
One Review for	Only Milo is a gold medal winner!


I am so glad that summer is finally here. Summer to me is sunshine, flowers in full bloom, warm weather, watermelon and ice cream; lots and lots of ice cream.
This is the time to get outside and enjoy nature. Time in nature has tremendous benefits. It is a surefire way to decrease stress in adults and kids. Nature is the best way to help everyone relax. Kids (and even adults) who have attention issues can find relief after being outside. Research has shown that adults and children are able to concentrate better, complete tasks and are more able to follow directions after they've spent time in a green setting.
Daydreaming is a lost art in our modern world, where we value productivity and achievement. However, most experts agree, that our brains need a break. Children and even adults can concentrate for just so long and then they need to space out. Not only that, goofing off or spacing out helps in fostering creativity in adults and certainly in our children. Summer time is the perfect time for absentmindedness. Gazing at the clouds, sitting barefoot in the grass, and watching bugs or birds, can help us refresh ourselves, reduce stress and get our minds working again.
There is so much to see in our neighborhoods. We are usually too much in a rush, or in our cars, to actually take note. Children view the world in a unique way, every rock, bush, police car and construction site can fascinate them. Take the time to see your neck of the woods through their eyes. Let them take the lead in showing you how to stop and appreciate your surroundings.
There is no child that does not love bubbles. It is a sure crowd pleaser. It is obviously best to do it outside so no one gets upset about the inevitable spills.
My kids loved this activity. I would buy some washable paint and we would collect rocks and then paint them. Even very young children can do this. Have some water on hand so you have an instant way to wash off and stay cool at the same time.
Kids love to tend a little plot of land and can help get your kids outside everyday, watering and weeding. Planting seeds and watching them grow is one of the simplest ways to appreciate G-d's world. If you are a newbie to gardening, you might want to plant some vegetables in large flowerpots. Tomatoes, cucumbers and squash plants grow pretty quickly, so your kids can easily see the fruit of their labors.
There you have it. 5 simple summer activities that will get you outside in no time.


text:
\section{Introduction}
The recent discovery \cite{atlasd, cmsd} of a scalar particle with properties
that are very similar to that of a Higgs boson completes the first stage of
the quest to understand the mechanism of electroweak symmetry breaking.
Indeed, after many years of preparation, ATLAS and CMS collaborations have
identified an elementary particle that may be directly connected to this
phenomenon.  Understanding this connection will be the primary focus of
particle physics in the coming years and there are two things that have to be
done. First, it is important to measure couplings of the Higgs boson  to gauge
bosons and fermions, and to verify that the Higgs couplings to various particles
are proportional to their masses.  Early measurements of the couplings
strengths seem to confirm this hypothesis \cite{atlasc}.  Second, it is
crucial to probe the Higgs boson self-interactions. Indeed, within the
Standard Model and many of its extensions, the Higgs boson self-interaction
triggers the electroweak symmetry breaking and it is important to verify that
we properly understand this phenomenon.

Self-interactions of the Higgs field and the electroweak symmetry breaking
induce the triple Higgs boson coupling. This coupling can be studied in the
production of a pair of Higgs bosons at the LHC \cite{bij,plehn,dj}.  At
leading order in QCD perturbation theory, the production of the Higgs boson
occurs in gluon fusion and proceeds either through a box $gg \to HH$ or a
triangle $gg \to H^*$ diagram, see Fig.~\ref{fig0}.  In the latter case the
off-shell Higgs boson decays to two Higgs bosons in the final state $H^* \to
HH$, making this contribution sensitive to triple Higgs boson coupling.
Unfortunately, observation of this process at the LHC is very challenging.
Indeed, it has a relatively small cross section to begin with and,
furthermore, it suffers from huge backgrounds that are present for almost all
major decay modes of the Higgs bosons.  Earlier estimates suggest that, with
$600~{\rm fb}^{-1}$, it is possible to study the double Higgs boson production
at the LHC in the $b \bar b \gamma \gamma$ channel \cite{baur}.  More recent
applications of jet substructure techniques to double Higgs production
indicate that one is sensitive to this process in $b \bar b W^+W^-$ and $ b
\bar b \tau \bar \tau $ channels with the integrated luminosity of $600
-1000~{\rm fb}^{-1}$ \cite{papa,dolan}.  Since substructure techniques are
still in the process of being developed, it is reasonable to expect
significant improvements in these initial estimates.  Therefore, we will
assume an optimistic outlook about prospects for measuring the double Higgs
boson production cross section at the LHC and we will try to improve the
quality of theoretical description of this process within the Standard Model.

We begin by summarizing what is known about the double Higgs boson production
in hadron collisions in the Standard Model.  As we already mentioned, the
dominant contribution to the process $pp \to HH$ is the gluon fusion that only
occurs at one-loop in perturbative QCD.  The corresponding partonic and
hadronic cross sections were computed in Refs.~\cite{bij,plehn}.  Part of this
contribution comes from $gg \to H^*$ process (see Fig.~\ref{fig0}) which is
equivalent to single Higgs boson production.  It is well-known that QCD
radiative corrections to single Higgs production are large
\cite{dawson,spira1,hnloexact}.  The bulk of these large radiative corrections
comes from relatively soft gluons that should not be sensitive to the details
of the final state as long as it is colorless. Therefore, we can expect that
similar large corrections are present in case of the double Higgs boson
production but, unfortunately, it is difficult to make this statement
precise. This is so because computation of QCD corrections to double Higgs
boson production requires four-point two-loop amplitudes with massive
particles which are out of reach of contemporary technology for perturbative
QCD computations.

\begin{figure}[t]
  \begin{center}
    \includegraphics[width=0.95\columnwidth]{figsgghh/LO.eps}
    \caption{Box and triangle diagrams that contribute to double Higgs boson
      production at leading order.  Solid lines refer to top quarks and
      dashed lines refer to Higgs bosons.  }
    \label{fig0}
  \end{center}
\end{figure}

Given this difficulty, computation of QCD corrections to double Higgs boson
production was performed in the approximation where the mass of the top quark
was taken to be very large compared to the partonic center-of-mass collision
energy and the Higgs boson mass \cite{Dawson:1998py}.  QCD corrections
obtained in this large-$M_t$ approximation appear to be significant; the ratio
of next-to-leading order cross section to leading-order cross section is close
to a factor two if factorization and renormalization scales are set to
$m_H$. However, it is unclear to what extent these large radiative corrections
are relevant for phenomenology because, as was repeatedly emphasized in the
literature \cite{Dawson:1998py,Dawson2013}, the large-$M_t$ approximation
fails to provide a good description of the $pp \to HH$ cross section for
realistic values of $M_t, m_H$ and the hadronic center-of-mass collision
energy.  To illustrate this point, we note that the large-$M_t$ limit of the
leading order cross section is about {\it fifty percent smaller} than the
exact leading-order cross section \cite{Dawson2013}.

To clarify to what extent the large radiative corrections observed in the
large-$M_t$ limit can be trusted, we decided to compute additional terms in the
$1/M_t$ expansion at next-to-leading order in perturbative QCD and to explore
how these power corrections affect the size of next-to-leading order
(NLO) QCD effects.  We note that it
was also found from comparisons of cross sections at leading order
\cite{Dawson2013}, that accounting for additional terms in $1/M_t$ expansion
does not  improve the agreement between expanded and exact results
for moderate and high values of the partonic center-of-mass energy
  $\sqrt{s}$.  In this situation, knowing additional terms in the expansion
may not help with the phenomenology {\it per se}, but it is still useful for
understanding the uncertainty that needs to be assigned to the NLO QCD
prediction for $pp \to HH$.  Moreover, if many terms in $1/M_t$ expansion are
available at next-to-leading order, we may try to improve on the quality of
the expansion by factoring out the exact leading order cross section. This
strategy is known to work very well in the case of single Higgs production in gluon
fusion, giving us a reason to believe that it will be useful for the
process $pp \to HH$ as well.  With the $1/M_t$ expansion at hand, we will be able
to determine the range of partonic center-of-mass energies, for which this procedure
works  well.

The remainder of this paper is organized as follows.  We explain  the computational methods in  Section~\ref{comp} and
describe numerical results  in Section~\ref{numres}.   We present our conclusions in Section~\ref{conc}.

\section{ Computational methods}
\label{comp}

In this Section we present technical details of  our  computation of the NLO QCD corrections to
Higgs boson pair production
in proton collisions, $pp \to HH$. The cross section
is  given by the product of parton distribution functions and the partonic cross section for
the process $ij \to HH$, where
$i$ and $j$ are the colliding partons
\begin{equation}
\sigma(pp \to HH +X) = \sum \limits_{ij} \int {\rm d} x_1 {\rm d} x_2  f_i(x_1) f_j(x_2) \sigma_{ij \to HH}.
\end{equation}
At leading order in the strong coupling constant,  both partons are gluons; at next-to-leading order,
quark-gluon and quark-antiquark  collisions start to contribute.

\begin{figure}[t]
  \begin{center}
    \includegraphics[width=0.6\columnwidth]{figsgghh/hadr_gghh0_exact_scut.eps}
    \caption{Leading order hadronic cross section for  Higgs boson pair production at the
    $14~{\rm TeV}$ LHC
    as the function of the upper cut on the Higgs boson pair invariant mass.
    Curve (b) is the full result; curve (a) is the box contribution;
    curve (c) is the
    triangle contribution.  The destructive interference between box and triangle contributions is apparent.
    We use MSTW2008 parton distribution functions \cite{mstw}.  }
    \label{figm1}
  \end{center}
\end{figure}

We take the gluon fusion channel $gg \to HH$ as an example to describe computational methods. At leading order, this process
occurs through a box diagram $gg \to HH$ or  through a triangle diagram $gg \to H^*$ with subsequent decay $H^* \to HH$,
see Fig.~\ref{fig0}.
Both the box and the triangle diagrams are mediated by the top quark loops.
Assuming   that the top quark mass $M_t$ is much larger than both, the mass of the
Higgs boson $m_H$  and the collision energy of the two gluons,
 we can understand the  leading contribution to $gg \to HH$ in this large-$M_t$ limit using the concept
of the effective Lagrangian. The effective Lagrangian
 for Higgs-gluon interaction can be obtained  by integrating out the top quark field from the Standard Model Lagrangian.
  It reads \cite{Dawson:1998py}
\be
{\cal L} = \frac{\alpha_s}{6\pi} {\rm Tr} \left [ G_{\mu \nu} G^{\mu \nu}\right ] \log \left ( 1+ \frac{H}{v} \right ),
\label{eq25}
\ee
where $G_{\mu \nu} = G_{\mu \nu}^{a} t^a$ is the gluon field-strength tensor and $v$ is the vacuum expectation value of the Higgs field.
Expanding Eq.~(\ref{eq25}) to second
order in $H/v$, we obtain terms that lead to  $gg H$ and $ggHH$ interactions.
The scattering amplitude  for $g(p_1) g(p_2) \to HH $, that follows from the effective Lagrangian
Eq.~(\ref{eq25}), reads
\be
{\cal A}_{\lambda_1 \lambda_2}  = \frac{\alpha_s \delta_{ab}}{8 \pi v} \delta_{\lambda_1 \lambda_2}
\left [
-\frac{4}{3} + \frac{4 m_H^2}{s-m_H^2}
\right ],
\label{eq1}
\ee where $s = 2p_1 \cdot p_2$, $\lambda_{1,2}$ are helicities of the two
gluons and $a,b$ are their color indices.  We note that the first term in
square brackets in Eq.~(\ref{eq1}) comes from the box diagram and the second
term from the triangle diagram, that contains a triple Higgs coupling.
It is interesting to note that box and triangle contributions to $gg \to HH$ amplitude  tend to
strongly cancel each other.  For example, at the partonic threshold $s = 4 m_H^2$, the
cancellation between the two contributions is exact. To further illustrate this point,  in Fig.~\ref{figm1}
we show the leading order Higgs boson pair  production cross section at the $14~{\rm TeV}$
LHC in dependence of the upper cut on the partonic center-of-mass collision energy.  As can be seen
from that Figure, the impact of the triple Higgs boson coupling on the observable
cross section comes from the destructive interference of the box and triangle contributions. It
reduces the cross section by almost a factor of two for a broad range of  $\sqrt{s_{\rm cut}}$
and implies  linear sensitivity of
the $pp \to HH$ production cross section to small changes in triple Higgs boson
coupling.  It also follows from Fig.~\ref{figm1}  that the $pp \to HH$  cross section gets saturated
at values of the Higgs pair invariant mass cut $\sqrt{s_{\rm cut}} \approx 600 \sim 700~{\rm GeV}$.
Therefore, for a reliable NLO computation, we require  accurate  description of partonic cross sections
for double Higgs boson production up to $\sqrt{s} \sim 600~{\rm GeV}$ since higher
partonic center-of-mass energies are not important for the hadronic $pp \to HH$ cross section.

While Eq.~(\ref{eq1}) is useful for thinking about Higgs boson production, it
does not lead to an adequate description of $pp \to HH$ cross section since
further terms in $1/M_t$ expansion are needed.  Deriving such terms is
straightforward at leading order in perturbative QCD where one can simply
obtain an exact result by computing the required one-loop
diagrams. Unfortunately, it becomes prohibitively difficult to do that at
next-to-leading order where computation of two-loop box diagrams for $gg \to
HH$ with full $M_t$-dependence is required.  To overcome this problem, we
expand the relevant NLO cross sections in powers of $1/M_t$.  We do so by
employing a procedure that has been used for the computation of finite-$M_t$
corrections to the production cross section of a single Higgs boson in gluon
fusion \cite{Pak:2009dg}.  In what follows we briefly describe it.

\begin{figure}[t]
\begin{center}
  \mbox{}\quad\quad\quad\includegraphics[width=0.95\columnwidth]{figsgghh/NLO1.eps}
  \\[3em]
  \includegraphics[width=0.95\columnwidth]{figsgghh/NLO2.eps}
  \\[2em]
  \caption{Examples of forward scattering amplitudes that we need to
    consider. Dashed vertical lines represent unitarity cuts. Solid lines
    are top  and light quarks,  dashed  lines are Higgs bosons.}
\label{fig0a}
\end{center}
\end{figure}

We start by representing the total cross section for the double Higgs boson
production by  the properly-normalized
discontinuity of the gluon forward scattering amplitudes (see Fig.~\ref{fig0a}
for sample Feynman diagrams),
\be
\sigma( gg \to HH) \sim {\rm Disc} \left [ {\cal A}_{gg \to gg} \right ]
\,.
\label{eq11}
\ee The discontinuity is obtained by cutting diagrams that contribute to
forward-scattering amplitudes through two Higgs lines at leading and
next-to-leading order, and through two Higgs lines and a gluon line at
next-to-leading order.  As explained in Ref.~\cite{am}, Eq.~(\ref{eq11}) is
helpful because the procedure of taking the discontinuity of the forward
scattering amplitude ${\cal A}_{gg \to gg} $ commutes with modern techniques
that can be used to compute it.  Indeed, to calculate diagrams that contribute
to ${\cal A}_{gg \to gg}$, we first perform the large-$M_t$ expansion by
treating masses and momenta of the Higgs bosons and, where appropriate, of a
cut gluon line, to be much smaller than the top quark mass.  Once this
expansion is carried out, we obtain a large number of Feynman integrals and we
reduce them to a minimal set of master integrals using the
integration-by-parts technique \cite{Tkachov:1981wb,Chetyrkin:1981qh}.  The
number of master integrals is small -- we require one integral for leading and
seven integrals for next-to-leading order computation.  The calculation proceeds
through a sequence of computer-algebra programs developed for computing mass
corrections to single Higgs boson production in gluon fusion
\cite{Pak:2009dg}.  Relevant three- and four-loop diagrams that contribute to
the forward scattering amplitude are obtained with {\sf QGRAF} \cite{qgraf},
supplemented with additional scripts to remove unnecessary diagrams.  Each
diagram is then expanded assuming $M_t^2 \gg m_H^2$ and $M_t^2 \gg s$ using
programs {\sf q2e} and {\sf exp} \cite{q2eexp}.  We express each Feynman
diagram as linear combination of scalar integrals using {\tt
  FORM}~\cite{Vermaseren:2000nd} and its parallel version {\tt
  TFORM}~\cite{Tentyukov:2007mu}.  The reduction to master integrals is
performed using {\tt FIRE}~\cite{Smirnov:2008iw,Smirnov:2013dia}\footnote{We
  thank A.V.~Smirnov and V.A.~Smirnov for allowing us to use the unpublished
  {\tt C++} version of {\tt FIRE}.}  which implements the Laporta
algorithm~\cite{laporta}. The first two expansion terms in $\rho$ are computed
for general QCD gauge parameter $\xi$ and the independence of the final result
of $\xi$ is used as a check of the computation. Furthermore, our result for
the $\rho^0$ contribution to the partonic cross section agrees with
Ref.~\cite{Dawson:1998py}.

Sample master integrals that appear at NLO are shown in Fig.~\ref{fig1}.  We
will discuss their computation in what follows. Note that we require these
master integrals to higher orders in the dimensional-regularization parameter
$\epsilon = (d-4)/2$ since they multiply the divergent reduction coefficients.
In principle, it is possible to derive exact expressions for these integrals
but this is cumbersome.  However, it is very easy to construct an expansion of
these integrals around the double Higgs partonic threshold to, essentially,
arbitrary order in the expansion parameter.  We now show how this is done for
individual master integrals.

For the leading order process $g(p_1) + g(p_2) \to H(p_3) +H(p_4)$,
there is just one master integral which corresponds to the available
phase space for final state particles \be I_0 =  \int [{\rm d} p_3
] [{\rm d} p_4] (2\pi)^d \delta^{(d)}(p_1 + p_2 - p_3 - p_4 ), \ee where
$[{\rm d} p] = {\rm d}^{d-1}p/((2\pi)^{(d-1)} 2 p_0)$, $p_1^2 = p_2^2 = 0$ and $p_3^2 = p_4^2 = m_H^2$.
At next-to-leading order, several different types of master integrals appear
since ${\cal O}(\alpha_s)$ corrections can either come from real gluon
emissions or from virtual gluon exchanges. For the real emission corrections,
four master integrals appear as the result of the reduction but only three of
them are linearly independent. For the virtual corrections, we need two-loop
vacuum bubble integrals and one additional master integral that we describe
below.

\begin{figure}[t]
  \begin{center}
    \includegraphics[width=0.95\columnwidth]{figsgghh/master.eps}
    \caption{The master integrals $I_1$, $I_2$, $I_3$, $I_4$ and $I_V$.
      Dashed lines cut through propagators that are replaced by the mass-shell
      conditions.  Dashed lines are the Higgs boson propagators and solid
      lines correspond to massless scalar propagators. In the
      case of $I_4$ the cross indicates a propagator raised to power minus
      one.  $I_V$ contributes to the virtual corrections at next-to-leading
      order.}
    \label{fig1}
  \end{center}
\end{figure}

The four  master integrals that we require to compute for the real emission corrections are
(see Fig.~\ref{fig1})
\be
\begin{split}
& I_1 = \int  [{\rm d} p_3 ] [{\rm d} p_4] [{\rm d} p_5]
(2\pi)^{d}\delta^{(d)}(p_1 + p_2 - p_3 - p_4 - p_5) , \\
& I_2 = \int  [{\rm d} p_3 ] [{\rm d} p_4] [{\rm d} p_5]
(2\pi)^{d}\delta^{(d)}(p_1 + p_2 - p_3 - p_4 - p_5)  \times ( (p_3+p_4)^2 - m_H^2), \\
& I_3 = \int  [{\rm d} p_3 ] [{\rm d} p_4] [{\rm d} p_5]
(2\pi)^{d}\delta^{(d)}(p_1 + p_2 - p_3 - p_4 - p_5)  \times ( p_2 - p_4)^2, \\
& I_4 = \int  [{\rm d} p_3 ] [{\rm d} p_4] [{\rm d} p_5]
(2\pi)^{d}\delta^{(d)}(p_1 + p_2 - p_3 - p_4 - p_5)  \times ((p_3+p_4)^2 - m_H^2)^{-1}.
\end{split}
\ee

To compute $I_1$, it is convenient to introduce integration over total
momentum of the two Higgs bosons $Q = p_3 + p_4$ by inserting ${\rm d}^dQ
\delta^{(d)}(Q -p_3 - p_4) = 1 $ into the integrand of $I_1$. We obtain
\be
  I_1 = \int \limits_{4 m_H^2}^{s} \frac{{\rm d} Q^2}{(2\pi)} {\rm
  Lips}(Q,p_3,p_4) {\rm Lips}(P_{12} , Q, p_5),
  \label{eq7}
\ee
where $P_{12} = p_1 + p_2$ and ${\rm Lips}$ is the two-particle
Lorentz-invariant phase space defined as
\be
{\rm Lips}(p,q,r) = \int [{\rm d} q] [{\rm d}  r] (2\pi)^d \delta^{(d)} ( p - q - r).
\ee
It is straightforward to compute the phase spaces that appear in  Eq.~(\ref{eq7}). We find
\be
\begin{split}
&  {\rm Lips}(Q,p_3,p_4) =  Q^{-2 \epsilon} \frac{\Omega_{d-1}
  2^{2\epsilon}}{(2\pi)^{d-2} 8}
\left ( 1 - \frac{4m_H^2}{Q^2} \right )^{1/2-\epsilon}, \\
& { \rm Lips}(P_{12},Q,p_5) =  s^{- \epsilon}
\frac{\Omega_{d-1} 2^{2\epsilon}}{(2\pi)^{d-1} 8} \left ( 1 - \frac{Q^2}{s} \right )^{1-2\ep},
\end{split}
\ee
where $s = P_{12}^2$ and $\Omega_{d} = 2\pi^{d/2}/\Gamma(d/2)$ is the solid angle of the $d$-dimensional space.
Combining the above formulas, we obtain
\be
I_1 = {\cal N} s^{-\ep}
\int \limits_{4 m_H^2}^{s} {\rm d} Q^2 Q^{-2\ep} \left ( 1 - \frac{4 m_H^2}{Q^2} \right )^{1/2-\ep}
\left ( 1 - \frac{Q^2}{s} \right )^{1-2\ep},
\label{eqi1q}
\ee
where the normalization factor ${\cal N}$ reads
\be
{\cal N} = \left [ \frac{\Gamma(1+\ep)}{(4\pi)^{d/2}} \right ]^2
\left [ 1 + 4 \epsilon + \left ( 12 - \frac{2\pi^2}{3} \right ) \ep^2
+ {\cal O}(\ep^3)
\right ].
\ee
To facilitate the computation of the integral, we change the integration variable by writing
$Q^2 = s ( 1- \delta \mu)$ and express the result in terms of the variable $\delta = 1 - 4m_H^2/s$.
We obtain
\be
I_1 = {\cal N} s^{1-2\ep} \delta^{5/2-3\ep}
\int \limits_{0}^{1}
\frac{{\rm d}\mu}{\sqrt{1-\delta \mu}} (1-\mu)^{1/2-\ep} \mu^{1-2\ep}.
\label{eqi12}
\ee
The integrand of $I_1$ can now be expanded in a Taylor series in $\delta$ and the resulting
integrals can be evaluated in a straightforward way.

We now discuss the evaluation of $I_2$. Note that the difference between $I_2$
and $I_1$ is due to additional terms in the integrand that, however, only
depend on $Q^2$ since $(p_3+p_4)^2 - m_H^2 = Q^2 - m_H^2$. Therefore, the
integral representation for $I_2$ can be easily deduced from
Eq.~(\ref{eqi1q}). We find
\be I_2 = {\cal N} s^{-\ep} \int \limits_{4
  m_H^2}^{s} {\rm d} Q^2 Q^{-2\ep} \left ( 1 - \frac{4 m_H^2}{Q^2} \right
)^{1/2-\ep} \left ( 1 - \frac{Q^2}{s} \right )^{1-2\ep} \times (Q^2 - m_H^2).
\label{eqi2q}
\ee
Trading  $Q^2$ for $\mu$, we obtain
\be
I_2 = {\cal N} s^{2-2\ep} \delta^{5/2-3\ep}
\int \limits_{0}^{1}
\frac{{\rm d} \mu}{\sqrt{1-\delta \mu}} (1 - \mu)^{1/2-\epsilon} \mu^{1-2\ep}
\left [ \frac{3}{4} + \delta \left ( \frac{1}{4} - \mu \right ) \right ],
\ee
and the Taylor expansion in $\delta$ becomes straightforward.

As the next step, we show that the integral $I_3$ is a linear combination of $I_1$ and $I_2$.  Indeed, since
\be
 I_3 =  \int  [{\rm d} p_3 ] [{\rm d} p_4] [{\rm d} p_5]
(2\pi)^{d} \delta^{(d)}(p_1 + p_2 - p_3 - p_4 - p_5)  ( m_H^2 - 2p_2 \cdot p_4 ),
 \ee
we can simplify it by using the following equations
\be
\int [{\rm d} p_3] [{\rm d} p_4 ]  (2\pi)^{d}\delta^{(d)}(Q - p_3 - p_4)  ( m_H^2 - 2 p_2 \cdot p_4)
= ( m_H^2 - p_2 \cdot Q ) {\rm Lips}(Q,p_3,p_4),
\ee
and
\be
\begin{split}
& \int [{\rm d} p_5 ][{\rm d} Q] (2\pi)^{d}\delta^{(d)}( P_{12} - p_5 - Q) ( m_H^2 - p_2 \cdot Q)\\
&= \int [{\rm d} p_5 ][{\rm d} Q] (2\pi)^{d}\delta^{(d)}( P_{12} -
p_5 - Q) \left ( m_H^2 - \frac{p_2 \cdot P_{12} ( s+Q^2)}{2s} \right )
\\
&= \left ( m_H^2 - \frac{s+Q^2}{4}  \right ) {\rm Lips}(P_{12},Q,p_5) .
\end{split}
\ee
Therefore, $I_3$ becomes
\be
I_3= {\cal N} s^{-\ep}
\int \limits_{4m_H^2}^{Q^2}
{\rm d}Q^2 Q^{-2\ep}
\left ( 1 - \frac{4m_H^2}{Q^2} \right )^{1/2-\ep}
\left ( 1 - \frac{Q^2}{s} \right )^{1-2\ep}
\left ( m_H^2 - \frac{s+Q^2}{4} \right ).
\ee
Using Eqs.~(\ref{eqi1q}) and~(\ref{eqi2q}),  it is easy to see that $I_3$ can be represented as a linear combination of $I_1$ and
$I_2$
\be
I_3 = \left ( m_H^2 - \frac{s}{4} \right ) I_1 - \frac{1}{4} (I_2 + m_H^2 I_1 ).
\ee

Finally, the integrand for $I_4$ differs from that for
$I_2$ because the term $(Q^2-m_H^2)$ occurs in
the denominator instead of the numerator;
therefore, the useful representation for $I_4$ can be easily derived following
the steps described above. We obtain
\be
I_4 = 4{\cal N} s^{-2\ep} \delta^{5/2-3\ep}
\int \limits_{0}^{1} \frac{{\rm d} \mu}{\sqrt{1-\delta \mu}}
\frac{(1-\mu)^{1/2-\ep} \mu^{1-2\ep}
}{3 + \delta (1 - 4\mu) },
\ee
and we can expand it in $\delta$ in a straightforward way.

Finally, additional master integrals are needed for the virtual corrections. The virtual corrections required for this
are the two-loop ones and their large-mass expansion leads to two distinct contributions. The first contribution arises
when the loop momenta are comparable to the mass of the top quark. In this case, the two-loop diagrams are
expandable in external momenta and the Higgs boson masses.  Using the integration-by-parts,
the two-loop integrals are mapped onto a single two-loop vacuum bubble integral.  In a situation where  one loop-momentum
is comparable to the top mass and the other loop-momentum is comparable to the Higgs boson mass or
to the partonic collision energy, a two-loop diagram factorizes
into a product of one-loop diagrams and we do not discuss it here.
In addition,  at next-to-leading order  diagrams appear where two Higgs bosons are produced in a way that involves
exchange of a gluon in a $t$-channel, see Fig.~\ref{fig0a}.
The computation of these diagrams requires a new  master integral. It reads
(see Fig.~\ref{fig1})
\be
I_V = \int [{\rm d} p_3] [{\rm d} p_4]  (2\pi)^d \delta(p_1+p_2 - p_3 - p_4) \times (p_1 - p_3)^{-2}.
\ee
We calculate it following the above discussion and  obtain
\be
I_V = - {\cal N}_V 8 \pi s^{-1-\ep}\delta^{1/2-\ep}
\int \limits_{0}^{1}
{\rm d} x \frac{x^{-\ep} (1-x)^{-\ep} (1+\delta) }{ (1+ \delta)^2 - 4 \delta (1-2 x)^2 },
\ee
where
\be
{\cal N}_V =  \frac{\Gamma(1+\ep)}{(4\pi)^{d/2}}
\left ( 1 - \frac{\pi^2}{6} \ep^2 + {\cal O}(\ep^3)
\right ) .
\ee
Expanding $I_V$  in $\delta$ is straightforward.

Once the reduction of the contributing diagrams to master integrals is performed
and once explicit expressions for master integrals are substituted, we obtain
unrenormalized results for partonic cross sections.  To obtain physical
results, we need to renormalize the strong coupling constant and the top quark
mass to remove the ultraviolet divergences, and to renormalize parton
distribution functions to remove the collinear singularities associated with
gluon emissions from the initial state.  For the ultraviolet renormalization,
we use the one-loop expressions
\be
\begin{split}
  \alpha_s^{\rm bare}  = \frac{\mu^{2\epsilon} \alpha_s}{S_\epsilon}
  \left ( 1 - \frac{\beta_0}{\epsilon} \frac{\alpha_s}{2\pi}  + \cdots \right ),
  \;\;\;\;
  M_{t}^{\rm bare } =  M_t
  \left [ 1 - \frac{C_F \alpha_s}{\pi S_\epsilon}
    \left( \frac{3}{4 \epsilon} - 1 - \frac{3}{4}\ln\frac{\mu^2}{M_t^2}\right) + \cdots \right ].
  \label{eq::ren}
\end{split}
\ee Here, $S_\epsilon = (4\pi)^{-\ep} e^{\gamma \epsilon}, \gamma =
0.5772\ldots$ is the Euler constant, $\alpha_s \equiv \alpha_s(\mu) $ is the
$\overline {\rm MS}$ QCD coupling constant evaluated at the scale $\mu$,
$\beta_0 = 11 N_c/6 - n_f/3$ is the one-loop QCD beta-function and $M_t$ is
the pole top quark mass.  For consistent ultraviolet renormalization,
we  first use $n_f=6$  but express our final result for cross section
through $\alpha_s$ with five
active flavours by using the one-loop decoupling relation for the top
quark. Ellipses in Eq.~(\ref{eq::ren}) stand for contributions suppressed by additional powers of
$\alpha_s$.

The collinear renormalization is performed in the standard way, by redefining
parton distribution functions.  The corresponding modification of the NLO
cross sections, required to make it finite, reads \be \sigma_{gg}^{(1)}(s) =
\delta {\bar \sigma}_{gg}^{(1)}(s) + \frac{1}{\ep}  \int \limits_{x_{\rm
    min}}^{1} {\rm d} x P_{gg}(x) \; \sigma_{gg}^{(0)} (x s), \ee where
$x_{\rm min} = 4 m_H^2/s$ is determined from the Higgs pair production
threshold in $gg$ collisions and $P_{gg}$ is the gluon splitting function
\be
P_{gg} = C_A \left [ \frac{1}{(1-x)_+} -1 + \frac{1-x}{x} + x(1-x) \right ]
+ \delta(1-x) \left ( \frac{11 C_A}{12} - \frac{n_f}{6} \right )\,,
\ee
with $C_A=3$ for QCD.  Similar equations hold also for $qg$, $\bar q g$ and
$q \bar q$ production channels; since they are standard, we do not present
them here.

\section{Numerical results}
\label{numres}

In this Section we present our results for the NLO QCD corrections to the
double Higgs boson production cross section at the LHC.  Values of the Higgs
boson mass and the on-shell top quark mass are taken to be $m_H
= 126~{\rm GeV}$~\cite{atlasd,cmsd} and $M_t = 173.18~{\rm
  GeV}$~\cite{Aaltonen:2012ra}, respectively.  We
begin with discussing partonic cross sections at leading and next-to-leading
order.  It is convenient to express the cross sections using two variables, $x
= 4 m_H^2/s = 1-\delta$ and $\rho = m_H^2/M_t^2$.  As we explained
in the previous Section, we compute the $HH$ production cross section as
series in $\rho = m_H^2/M_t^2$.
 The expansion starts at $\rho^{0}$ and we are able to obtain
five  terms of the $\rho$-expansion, up to ${\cal O}(\rho^4)$, for the $gg$
partonic channel and seven terms, up to ${\cal O}(\rho^6)$, for the $qg$ and $q
\bar q$ channel.  The master integrals are computed as an expansion in the
parameter $\delta = 1-x$; for the final results all terms up to ${\cal O}(\delta^{50})$
are included.
The partonic cross sections are defined as
\be
\sigma_{ij \to H+X}(s,\rho) =
 \delta_{ig} \delta_{jg} \sigma_{gg}^{(0)}(s,\rho) + \frac{\alpha_s}{\pi}\sigma^{(1)}_{ij}(s,\rho),
\ee
where $\sigma^{(1)}_{ij}$ is the ${\cal O}(\alpha_s)$ correction to the leading
order cross section.
For the discussion of the partonic cross sections,  we set the factorization
and the renormalization scales to $ \mu_r = \mu_f = 2 m_H$. We will describe the scale
dependence of our results below when we consider the hadronic cross section.

\begin{figure}[t]
  \begin{center}
    \includegraphics[width=0.48\columnwidth]{figsgghh/part_gghh0.eps}
    \includegraphics[width=0.48\columnwidth]{figsgghh/part_gghh1_expa.eps}
    \caption{Leading order partonic $gg \to HH$ cross section (left pane) and
      next-to-leading order {\it contribution} to $gg \to HH$ cross section
      $\alpha_s/\pi \times \sigma_{gg}^{(1)}$ (right pane), in
      fb. Different lines correspond to 1) exact leading order cross section
      -- black solid; 2) cross sections expanded
      to ${\cal O}(\rho^0)$ -- short-dashed red;
      to ${\cal O}(\rho^1)$ -- short-dashed green;
      to ${\cal O}(\rho^2)$ -- dashed orange;
      to ${\cal O}(\rho^3)$ -- dashed blue;
      to ${\cal O}(\rho^4)$ -- dashed violet;
      to ${\cal O}(\rho^5)$ -- long-dashed light gray;
      to ${\cal O}(\rho^6)$ -- long-dashed dark gray;
      See text for the description of
      input parameters. }
\label{fig3}
\end{center}
\end{figure}

We begin by showing some  results for the $gg$  channel.  In Fig.~\ref{fig3} we compare
$\sigma_{gg}^{(0)}(s,\rho)$  with seven approximate cross sections   that are obtained  by expanding $\sigma_{gg}^{(0)}$
in $\rho$ through ${\cal O}(\rho^{i})$, $i=0,\ldots,6$.
It is clear from Fig.~\ref{fig3} that  the convergence
of the expansion is poor. Indeed, already at $\sqrt{s} \sim  350~{\rm GeV}$,
there is a sizable difference  between the exact and the expanded result.
In the right pane of Fig.~\ref{fig3} we show the NLO contribution
to the cross section expanded to different orders in $\rho$.   Similar to the leading order case,
the $1/M_t$ expansion does not appear to converge.

\begin{figure}[t]
  \begin{center}
    \includegraphics[width=0.48\columnwidth]{figsgghh/part_gghh1_fact.eps}
    \includegraphics[width=0.48\columnwidth]{figsgghh/part_qghh1_fact.eps}
    \\
    \includegraphics[width=0.48\columnwidth]{figsgghh/part_qbhh1_fact.eps}
    \caption{ Next-to-leading order contribution to $gg \to HH$, $qg \to HH$
      and $q \bar q \to HH$ cross sections re-scaled by exact leading order
      result, in fb. The color coding is as in Fig.~\ref{fig3}.}
    \label{fig4}
  \end{center}
\end{figure}

The bad convergence of the $1/M_t$ expansion should not be very
surprising. Indeed, we note that the expansion is not supposed to work beyond,
or even close to, the top quark threshold that occurs at $\sqrt{s} = 2 M_t$.
Therefore, using the expansion techniques described above, we can only hope to
obtain reliable results for values of $s \ge 4 M_t^2$ if we can show that
corrections do not strongly depend on $s$.  From this perspective, the
situation is similar to what occurs in the single Higgs boson production in
gluon fusion where the applicability of radiative corrections computed in the
large-$M_t$ approximation is usually extended by combining them with the {\it exact}
leading order cross section for $gg \to H$.  The validity of such an approach
in single Higgs production is verified by comparing it to the exact results at
NLO \cite{hnloexact} and by its consistency with known power corrections to
the large-$M_t$ limit at NNLO QCD
\cite{powerc1,powerc2,Pak:2009dg,Pak:2011hs,powerc4}.  Motivated by the
success of this approach to QCD corrections in single Higgs boson production,
we apply it to Higgs pair production as well.  We write the NLO QCD
contribution to the partonic cross section as
\be
\label{eqnlo}
\sigma_{ij,N}^{(1)} =
\sigma_{gg,\rm exact}^{(0)}  \Delta_{ij}^{(N)},
\;\;\;\;\;  \Delta_{ij}^{(N)} =
\frac{\sigma_{ij,\rm exp}^{(1)}}{\sigma_{gg,\rm exp}^{(0)}} =
\frac{\sum \limits_{n=0}^{N} c_{ij,n}^{\rm NLO}\rho^n}{\sum \limits_{n=0}^{N} c_{gg,n}^{\rm LO}\rho^n} ,
\ee
where both numerator and denominator of the $\Delta$-factor
are expanded to the same order in $\rho$. By changing $N$ in
the above formula, we can check the stability of our computation against  additional power corrections.
Ideally, $\Delta_{ij}^{(N)}$,  should become $N$-independent, after sufficient number of terms are included in the numerator and
denominator in Eq.~(\ref{eqnlo}).

\begin{figure}[t]
  \begin{center}
    \includegraphics[width=0.48\columnwidth]{figsgghh/hadr_gghh0_scut.eps}
    \includegraphics[width=0.48\columnwidth]{figsgghh/hadr_gghh1_scut.eps}
    \\
    \includegraphics[width=0.48\columnwidth]{figsgghh/hadr_qghh1_scut.eps}
    \includegraphics[width=0.48\columnwidth]{figsgghh/hadr_qbhh1_scut.eps}
    \caption{ Leading and next-to-leading order contributions to hadronic
      production cross sections of Higgs boson pairs. Different curves
      represent  the cross section obtained through expansion to different
      orders in $\rho$; rescaling by the leading order cross section is always
      included. The color coding is as in Fig.~\ref{fig3}.}
    \label{fig5}
  \end{center}
\end{figure}

Our results for $\sigma_{gg,N}^{(1)}$ are shown in Fig.~\ref{fig4}. We see
that for $N=0,1,2,3,4$, $\sigma_{gg,N}^{(1)}$ is fairly stable over a broad
range of partonic center-of-mass energies.  In fact, there is practically no
difference between $\sigma_{gg,2}^{(1)}$ and $\sigma_{gg,3}^{(1)}$ all the way
up to $\sqrt{s} \sim 600~{\rm GeV}$ but, unfortunately, $\sigma_{gg,4}^{(1)}$
shows a $13$ percent increase relative to $\sigma_{gg,3}^{(1)}$ for $\sqrt{s}
\sim 450~{\rm GeV}$.  The situation is similar for the $qg$ channel and it is
much worse for $q \bar q$ channel where even with as many as seven terms of
the $1/M_t$ expansion the convergence seems poor, see Fig.~\ref{fig4}.  To
understand the differences between partonic channels, we note that the leading
order cross section $\sigma_{gg}^{(0)}$ does not properly describe the
kinematic features of $\sigma_{qg}^{(1)}$ and $\sigma_{q \bar q}^{(1)}$.
Indeed, the $qg $ scattering, for example, mainly occurs through a $t$-channel
gluon exchange which, for large $s$, has little to do with the
leading order process of a gluon fusion into a pair of Higgs bosons.
Fortunately, these subtleties do not impact predictions for hadronic cross
sections because the $qg$ and $q \bar q$ channels are numerically small --
they provide at most ten percent correction to the next-to-leading order
contribution to Higgs boson pair production cross section. Therefore, even
relatively low accuracy for $q g$ and $q \bar q$ channels is sufficient for
reliable phenomenology.

We proceed now to the discussion of hadronic cross sections.  To obtain numerical results  shown below we employ
MSTW2008  parton distribution functions (PDFs) \cite{mstw}.
We consistently use leading order PDFs to compute leading order cross sections
and next-to-leading order PDFs to compute next-to-leading order cross sections.   We assume the energy of the LHC
to be $14~{\rm TeV}$.   Values of the strong coupling constants
$\alpha_s(M_{\rm Z})$ that we use
in our computation are obtained from the MSTW PDF fit. Their leading and next-to-leading order values are
$0.139384$ and $0.120176$, respectively.

We  present  results for hadronic cross sections
as a function of the upper cut on the partonic center-of-mass energy $\sqrt{s_{\rm cut}}$.
This allows us to explore the stability of the  $1/M_t$ expansion of the Higgs boson pair
production cross section as we move from the threshold region, where this expansion works
well, to the high-energy region where this expansion becomes less reliable.
We can also use this cut  as a proxy for the  Higgs boson pair invariant mass
 cut  which  may be useful  for enhancing observability of  the triple Higgs  boson coupling.  We note
that at leading order in QCD, a cut on partonic center of mass energy
is equivalent to the cut on the invariant mass of the Higgs boson pair while at next-to-leading order  the equivalence is not exact anymore.
For all results below, we use the NLO contributions to partonic cross sections
re-scaled with exact leading order cross section, cf. Eq.~(\ref{eqnlo}).

Our results for leading and next-to-leading order contributions to hadronic
cross sections are shown in Fig.~\ref{fig5}.  The NLO QCD predictions for
hadronic cross sections appear to be more reliable than similar results for
partonic cross sections; the reason for this is the known enhancement of gluon
luminosity at small values of $s$ which reduces contributions of large-$s$
partonic processes to hadronic cross sections.  To illustrate this point, we
note that even for $\sqrt{s_{\rm cut}} \sim 700~{\rm GeV}$, the shift in
$\delta \sigma_{gg}^{\rm NLO}$ due to the last computed term in the $1/M_t$
expansion is close to twelve percent. For lower values of $\sqrt{s_{\rm cut}}$
the convergence is significantly better; for $\sqrt{s_{\rm cut}} \sim 450~{\rm
  GeV}$, a similar shift is close to seven percent.  We note that these numbers
refer to NLO contributions to next-to-leading order cross sections and that the
numerical significance of these shifts is further ameliorated by large leading
contribution.

 \begin{figure}[t]
  \begin{center}
    \includegraphics[width=0.48\columnwidth]{figsgghh/hadr_k_scut.eps}
    \includegraphics[width=0.48\columnwidth]{figsgghh/part_k_ssm2mh.eps}
    \caption{ The NLO $K$-factors defined as the ratio of NLO and LO hadronic
      (left) and partonic (right) cross sections are shown as the function of
      $\sqrt{s_{\rm cut}}$.  The renormalization and factorization
      scales are chosen to be $\mu = 2 m_H$. The color coding is as in
      Fig.~\ref{fig3}.}
    \label{fig7}
  \end{center}
\end{figure}

As we already mentioned in the Introduction, QCD corrections to  Higgs boson pair
production cross section
at the LHC are  large. To illustrate this,
in the left pane of Fig.~\ref{fig7} we show the $K$-factor,  defined as the ratio of NLO and LO
 $pp \to HH+X$ cross sections, evaluated
at $\mu = 2m_H$, as a function  of $\sqrt{s_{\rm cut}}$.
In general, the $K$-factors are large, confirming earlier
observation of Ref.~\cite{Dawson:1998py}.  However, the $K$-factor  is also
strongly dependent on $s_{\rm cut}$,  decreasing  significantly  from
the threshold region $\sqrt{s_{\rm cut}} \approx 2 m_H$ to large values of $s_{\rm cut}$.
This change of the $K$-factor
is related to additional suppression of the leading order
cross section for $gg \to HH$ in the threshold region that we
mentioned in the Introduction and the fact that for the NLO amplitude such suppression  is not present.
Because of that, the $K$-factor in the threshold
region is enhanced.  To illustrate this point, we show the partonic $gg$ cross section expanded to
first non-vanishing orders in $\rho$ and $\delta$ at leading and next-to-leading order in the threshold
region\footnote{The ${\cal O}(\rho^0)$ leading order partonic cross section scales as $\delta^{5/2}$
at threshold.}
\begin{align}
  & \sigma_{gg} \approx \frac{G_F^2  m_H^2}{2\pi}
  \left ( \frac{\alpha_s}{\pi} \right )^2 \left \{
      \frac{7 \rho }{25920} \delta^{3/2}
      + \rho^2 \left(
        \frac{49}{4147200}\delta^{1/2}
        + \frac{24001}{87091200}\delta^{3/2}
      \right)
    \right.
    \nonumber\\&\mbox{}
    \left.
    +
    \frac{\alpha_s}{\pi}
    \left [
      - \frac{\delta^{3/2}}{1296}
      + \rho \left (
        -\frac{7}{103680} \sqrt{\delta}
        + \delta^{3/2} \left\{ \frac{8957}{466560}
          - \frac{7 \pi^2}{25920}
          + \frac{7}{1620}\lmmh
          + \left (-\frac{7}{270}
        \right.\right. \right. \right. \right.
        \nonumber\\ & \left. \left. \left. \left. \left.
            - \frac{7}{2160} \ln \frac{\mu^2}{m_H^2}
          \right  ) \ln 2 + \frac{7}{540} \ln^2 2
          + \left  (- \frac{7}{810}
            + \frac{7}{720} \ln 2
            - \frac{7}{4320} \ln \frac{\mu^2}{m_H^2}
          \right ) L_\delta  +
          \frac{7}{4320}  L_\delta^2
        \right \}
      \right  )
      \right.\right.  \nonumber\\&\mbox{} \left.\left.
      + \rho^2 \left(
        \left\{
          \frac{128399}{261273600}
          - \frac{49}{4147200} \pi^2
          + \frac{49}{345600}\lmmh
          + \frac{49}{86400}\ln^2 2
          + \frac{49}{691200} L_\delta^2
        \right.\right.\right.\right.  \nonumber\\&\mbox{} \left.\left. \left.\left.
          + \left(
            - \frac{49}{57600}
            - \frac{49}{345600}\lmmh
          \right)\ln 2
          + \left(
            - \frac{49}{172800}
            - \frac{49}{691200}\lmmh
            + \frac{49}{115200}\ln 2
            \right) L_\delta
        \right\}\delta^{1/2}
        \right.\right.\right.  \nonumber\\&\mbox{} \left.\left.\left.
        +\left\{
          \frac{318919}{15676416}
          - \frac{24001}{87091200} \pi^2
          + \frac{193037}{43545600}\lmmh
          + \frac{24001}{1814400}\ln^2 2
        \right.\right.\right.\right.  \nonumber\\&\mbox{} \left.\left. \left.\left.
          + \frac{24001}{14515200} L_\delta^2
          + \left(
            - \frac{24001}{907200}
            - \frac{24001}{7257600}\lmmh
          \right)\ln 2
        \right.\right.\right.\right.  \nonumber\\&\mbox{} \left.\left. \left.\left.
          + \left(
            - \frac{382987}{43545600}
            - \frac{24001}{14515200}\lmmh
            + \frac{24001}{2419200}\ln 2
            \right) L_\delta
        \right\}\delta^{3/2}
      \right)
    \right ] + \ldots \right \}
\end{align}
where $L_\delta = \ln \delta$ and ellipses stand for terms additionally
suppressed by powers of either $\rho$ or $\delta$.  We observe that in the
limit $\delta \to 0$, dominant contributions to $\sigma_{gg}$ come from a term
${\cal O}(\alpha_s^2 \rho^2 \sqrt{\delta})$ at leading order and from a term $
{\cal O}(\alpha_s^3 \rho^2 \sqrt{\delta} \ln \delta^2)$ at next-to-leading
order.  This implies that the behavior of the $K$-factor in the $\delta \to 0$
limit is strongly affected by power-suppressed $1/M_t$ terms and that the
$K$-factor becomes infinite at the exact $\delta \to 0$ threshold for $HH$
production.  This point is further illustrated in the right pane of
Fig.~\ref{fig7}, where {\it partonic} $K$-factors are shown in the vicinity of
the two-Higgs threshold.  It follows from that plot that the threshold limit
of the ${\cal O}(\rho^{0,1})$ curves is significantly different from the
approximation that includes ${\cal O}(\rho^2)$ and higher-power corrections.
We also note that $1/M_t$-corrections change the hadronic $K$-factor by about
$14$ percent at $\sqrt{s_{\rm cut}} = 700~{\rm GeV}$ and the change decreases
for smaller values of $s_{\rm cut}$.  The shift in the $\sqrt{s_{\rm cut}} =
700~{\rm GeV}$ $K$-factor due to the last computed $1/M_t$ correction is close
to seven percent.

\begin{figure}[t]
  \begin{center}
    \includegraphics[width=0.5\columnwidth]{figsgghh/hadr_gghh01_mu.eps}
    \caption{ Scale dependence of the hadronic production cross section for
      $pp \to HH$.  }
    \label{fig6}
  \end{center}
\end{figure}

In Fig.~\ref{fig6}, we show the residual dependence of the production cross
section $pp \to HH$ on the factorization and renormalization scales that we
set equal to each other.  The NLO cross section is computed with all available
$1/M_t$ corrections included.  The cut on the partonic center-of-mass
collision energy of $600~{\rm GeV}$ is imposed.  It follows from
Fig.~\ref{fig6} that the NLO QCD cross section is practically independent of
the renormalization and factorization scales in a broad range of $\mu$.
Choosing $\mu = 2m_H$ as the central value and estimating the
uncertainty by increasing and decreasing $\mu$ by a factor of two, we arrive
at the NLO cross section estimate $\sigma_{pp \to HH} = 38^{+0}_{-2}~{\rm fb}$
for $\sqrt{s_{\rm cut}} = 600~{\rm GeV}$ to be compared to $\sigma_{pp \to HH}
= 18^{+6}_{-4}~{\rm fb}$ at LO. The scale-dependence uncertainty of the NLO
cross section is therefore close to five percent, a significant improvement
compared to ${\cal O}(30\%)$ uncertainty of the leading order cross section.

\begin{figure}[t]
  \begin{center}
    \includegraphics[width=0.5\columnwidth]{figsgghh/hadr_all_scut.eps}
    \caption{The NLO hadronic cross section at the $14~{\rm TeV}$ LHC as a
      function of $\sqrt{s_{\rm cut}}$.  Two black curves correspond to $\pm
      20\%$ variation in the triple Higgs boson coupling relative to its SM
      value.  The violet (hatched) band shows the uncertainty in the SM prediction for
      $pp \to HH$ due to uncalculated $1/M_t$ corrections.  }
    \label{fig8}
  \end{center}
\end{figure}

Finally, we briefly discuss implications of our results for the extraction of
the triple Higgs boson coupling by comparing variations in $pp \to HH$ cross
section induced by changes in $\lambda_{HHH}$ and the uncertainties in the
Standard Model prediction for that cross section.  In particular, we focus on
the uncertainties caused by imperfect knowledge of the $1/M_t$ corrections to
the cross section.  For our best estimate of the $pp \to HH$ cross section, we
use exact leading order result and next-to-leading contributions expanded to
highest known power in $\rho$ (i.e. $\rho^4$ for $gg$ channel and $\rho^6$ for
$qg$ and $q \bar q$ channel).  We assign the one-sided error to this cross
section by comparing it with a similar computation that employs NLO cross
sections expanded through $\rho^3$ in $gg$ channel and $\rho^6$ in $qg$ and $q
\bar q$ channels.  In Fig.~\ref{fig8} we show the NLO QCD cross sections for
double Higgs boson production for three values of triple Higgs boson coupling,
as a function of the cut on partonic center-of-mass energy.  Two black curves
correspond to $\pm 20\%$ variations in the triple Higgs boson coupling; such
variations cause ${\cal O}(20\%)$ changes in the cross section since, as we
discussed in the Introduction, the impact of the triple Higgs boson coupling
on the $pp \to HH$ cross section is caused by the destructive interference of
box and triangle contributions.  The violet (hatched) band shows Standard Model (SM)
prediction for $pp \to HH$ including the uncertainty of the $1/M_t$ expansion.
We conclude from Fig.~\ref{fig8} that the quality of our current knowledge of
the Higgs boson pair production cross section, inasmuch as $1/M_t$ corrections
are concerned, is sufficient to detect ${\cal O}(10 \%)$ deviations in Higgs
triple boson coupling, relative to its Standard Model value.

\section{Conclusions}
\label{conc}

In this paper, we studied top quark mass corrections to the production cross
section of the Higgs boson pair at the LHC through next-to-leading order in
perturbative QCD. This is an interesting process since it allows us to directly explore
the self-interaction potential of the Higgs field.
QCD corrections to Higgs boson
pair production are known to be very large \cite{Dawson:1998py}; they enhance
the Higgs pair production cross section by almost a factor two.  For technical
reasons, these corrections were originally computed \cite{Dawson:1998py} in
the infinite top quark mass approximation which, for realistic Higgs boson
masses, has very limited applicability.  For phenomenological applications, it
is important to check the stability of this result against $1/M_t$ power
corrections.  Computation of such mass corrections at next-to-leading order in
QCD is the main goal of this paper.

We calculated power corrections through ${\cal O}(1/M_t^8)$ for $gg \to HH$
partonic channel and through ${\cal O}(1/M_t^{12})$ for $q g$ and $q \bar q$.
These corrections turned out to be large and poorly convergent which is hardly
surprising since similar behavior can be observed already at leading order,
where many terms in $1/M_t$ expansion can be compared to the exact result.  We
have shown that the problem of poor convergence can be cured if the exact
leading-order cross section is used to normalize the NLO QCD corrections.
With such normalization, we find that mass corrections provide ${\cal O}(10\%)$
increase in the NLO QCD prediction for $pp \to HH$ production cross section.

Our computation provides a realistic estimate of the NLO QCD effects in the
total cross section for a Higgs boson pair production.  It justifies the use
of the large-$M_t$ approximation to describe QCD corrections to this process
and opens up a way to reliably estimate NNLO QCD corrections to $pp \to
HH$.\footnote{Very recently,
  next-to-next-to-leading order soft and
  virtual corrections were computed in
  this limit~\cite{deFlorian:2013uza}.}
Given a very small dependence of the cross section on the renormalization
and factorization scales, which may appear to be accidental given the
magnitude of the NLO QCD corrections, computation of NNLO QCD corrections is
important for quantifying theoretical uncertainty in $\sigma(pp \to HH)$.
Moreover, it is worth remembering that observation of $pp \to HH$ is difficult
and requires good control of kinematic properties of Higgs bosons decay
products. It remains an important and challenging problem to extend NLO QCD
results presented in this paper to describe kinematic distributions relevant
for $pp \to HH$ observation.

\medskip

\noindent
{\bf Acknowledgments}

The research of J.H, J.G. and M.S. is supported by the Deutsche Forschungsgemeinschaft in the
Sonderforschungsbereich Transregio~9 ``Computational Particle Physics''.
The  research of K.M. is partially supported by US NSF under grants PHY-1214000.
The research of K.M. and J.G. are partially supported  by Karlsruhe Institute of Technology through
is distinguished researcher fellowship program.

\medskip

\noindent

redpajama_set_name: RedPajamaArXiv


text:
package com.example;

import org.seasar.doma.*;
import org.seasar.doma.boot.ConfigAutowireable;
import org.seasar.doma.jdbc.Result;
import org.springframework.transaction.annotation.Transactional;

import java.util.List;

/**
 * Created by shigeru on 17/05/05.
 */
@ConfigAutowireable
@Dao
public interface ReservationDao {
    @Select
    List<Reservation> selectAll();

    @Select
    List<Reservation> selectByName(String name);

    @Select
    Reservation find(int id);

    // @Insert(sqlFile = true)
    @Insert
    @Transactional
    Result<Reservation> insert(Reservation reservation);
    // int insert(Reservation reservation);

    @Update(sqlFile = true)
    @Transactional
    Result<Reservation> update(Reservation reservation);
    // int update(Reservation reservation);

    @Delete(sqlFile = true)
    @Transactional
    Result<Reservation> delete(Reservation reservation);
    // int delete(Reservation reservation);
}


Providing optimal comfort, convenience, and hygiene to your eyes, Focus Dailies disposable contacts provide fresh, clean contacts at the start of each day, eliminating daily lens cleansing and reducing the chance of deposit build-up. Ideal for people with allergies, or for those with a busy or irregular lifestyle, Focus Dailies are the easiest, most care-free, and most comfortable option of contact lenses you can subscribe to. In addition, they use a patented light Stream technology for even clearer vision.


text:
namespace CloudFlare.NET
{
    using System;
    using System.Collections.Generic;
    using System.Diagnostics;
    using System.Linq;
    using Newtonsoft.Json;

    /// <summary>
    /// A Zone is a domain name along with its subdomains and other identities.
    /// </summary>
    /// <seealso href="https://api.cloudflare.com/#zone-properties"/>
    [DebuggerDisplay("{DebuggerDisplay,nq}")]
    public class Zone : IIdentifier, IModified
    {
        private static readonly IReadOnlyList<string> EmptyStrings = new string[0];

        /// <summary>
        /// Initializes a new instance of the <see cref="Zone"/> class.
        /// </summary>
        public Zone(
            IdentifierTag id,
            DateTimeOffset? createdOn,
            DateTimeOffset modifiedOn,
            string name,
            int developmentMode,
            IReadOnlyList<string> originalNameServers = null,
            string originalRegistrar = null,
            string originalDnshost = null,
            IReadOnlyList<string> nameServers = null,
            ZoneStatusType status = ZoneStatusType.active)
        {
            if (id == null)
                throw new ArgumentNullException(nameof(id));
            if (string.IsNullOrWhiteSpace(name))
                throw new ArgumentNullException(nameof(name));

            Id = id;
            CreatedOn = createdOn;
            ModifiedOn = modifiedOn;
            Name = name;
            DevelopmentMode = developmentMode;
            OriginalNameServers = originalNameServers ?? EmptyStrings;
            OriginalRegistrar = originalRegistrar ?? string.Empty;
            OriginalDnshost = originalDnshost ?? string.Empty;
            NameServers = nameServers ?? EmptyStrings;
            Status = status;
        }

        /// <summary>
        /// API item identifier tag.
        /// </summary>
        public IdentifierTag Id { get; }

        /// <summary>
        /// When the zone was created.
        /// </summary>
        public DateTimeOffset? CreatedOn { get; }

        /// <summary>
        /// When the zone was last modified.
        /// </summary>
        public DateTimeOffset ModifiedOn { get; }

        /// <summary>
        /// The domain name.
        /// </summary>
        [JsonProperty("name")]
        public string Name { get; }

        /// <summary>
        /// The interval (in seconds) from when development mode expires (positive integer) or last expired (negative
        /// integer) for the domain. If development mode has never been enabled, this value is 0.
        /// </summary>
        [JsonProperty("development_mode")]
        public int DevelopmentMode { get; }

        /// <summary>
        /// Original name servers before moving to CloudFlare.
        /// </summary>
        [JsonProperty("original_name_servers")]
        public IReadOnlyList<string> OriginalNameServers { get; }

        /// <summary>
        /// Registrar for the domain at the time of switching to CloudFlare.
        /// </summary>
        [JsonProperty("original_registrar")]
        public string OriginalRegistrar { get; }

        /// <summary>
        /// DNS host at the time of switching to CloudFlare.
        /// </summary>
        [JsonProperty("original_dnshost")]
        public string OriginalDnshost { get; }

        /// <summary>
        /// CloudFlare-assigned name servers. This is only populated for zones that use CloudFlare DNS.
        /// </summary>
        [JsonProperty("name_servers")]
        public IReadOnlyList<string> NameServers { get; }

        /// <summary>
        /// Status of the zone.
        /// </summary>
        [JsonProperty("status")]
        public ZoneStatusType Status { get; }

        private string DebuggerDisplay => $"{GetType().Name}: {Name}";
    }
}


BOWLING GREEN, Ohio - The No. 9 ranked Bowling Green State University hockey team took game one of their two game series against Ferris State University on Friday (Jan. 25) night as the Falcons defeated the Bulldogs by a final score of two to zero. The Falcons scored twice on 37 shots on goal. Sophomore goaltender Eric Dop recorded his second shutout victory in a row as he backstopped the Falcons to victory. This is the third shutout of his career and his second shutout victory. All three shutouts have been recorded during the 2018-19 season. Dop's goaltending would remain strong throughout the contest as fellow sophomores Max Johnson and Cameron Wright would score a pair of power play goals for Bowling Green. Bowling Green will be back on home ice on Saturday (Jan. 26) night as they host the Bulldogs for the second of this two game series.
- Max Johnson would tally the first goal of the evening on a BGSU power play 15:35 into the second period. This turned out to be the game-winner. He was assisted by Brandon Kruse and Stephen Baylis.
- Cameron Wright would score another power play goal for the Falcons 10:29 into the third period. Max Johnson and Alec Rauhauser would record assists on the play.
- Eric Dop's 22 save shutout in Friday's (Jan. 25) win is the third shutout of his season and career. This is his second shutout victory in a row as Eric Dop made 31 saves to defeat the Alaska Nanooks last weekend (Jan. 19). This is the first time Bowling Green has recorded multiple shutouts in a row since the 2016-17 season when the Falcons recorded three straight shutout wins to close the regular season (Feb. 11, 24, 25, 2017). Chris Nell was in net for BGSU in those three games. One more shutout for Eric Dop would tie him with fellow Falcon goaltender Ryan Bednard with four in his career.
- Max Johnson tallied multi-point game number 14 of his career in Friday (Jan. 25) night's win. He now has seven multi-point performances on the 2018-19 campaign.
- Cameron Wright tallied his sixed goal of the season in Friday's (Jan 25) win. This goal was Wright's 40th career point for the Bowling Green Falcons. He has recorded six goals and nine assists for 15 points on the season.
- Tallying an assist each, Stephen Baylis and Brandon Kruse both extended their point streaks to two games apiece. This is Brandon Kruse's third multi-game point streak of the 2018-19 season, as he has had streaks of six games and seven games respectively.
- Bowling Green's win over Ferris State keeps them in second place in the Western Collegiate Hockey Association standings with 40 points. They are just five points behind Minnesota State who sit in first place with 45 points.
- Bowling Green will host the Ferris State Bulldogs for game two of this series on Saturday (Jan. 26) night. The Falcons will then continue WCHA play as they travel to Northern Michigan next weekend for a two game road series (Feb. 1-2).


text:
Chip In Here!
Periodic Email News
Carroll County NH Dems!
Town Committees
Greater Ossipee Democrats
Iron Mtn. Democrats (Bartlett, Jackson & Hart's Location)
Moose Mountain Area Democrats (Wakefield & Brookfield)
Tri-Town Democrats (Moultonborough, Tuftonboro & Sandwich)
Conway Democrats
Wolfeboro Democrats
Knirk column – "Liberty & Responsibility"
Ten Things to Know — 11/16/21
Learn About the Free Staters on November 16 at Tri-Town DEMs
Mike Cryans to Visit Great Ossipee DEMs on November 22 via Zoom!
Everyone Should Have the Chance to Vote With Ease
Events December 30, 2021 December 30, 2021 Carroll County Democrats
The pandemic and how we as a national community are trying to fight it has become a political issue due to the most right-wing members go the GOP and the enabling of those right wingers by the self-proclaimed centrist or moderate GOP members like Karen Umberger (GOP Rep of Conway) and Mark McConkey (GOP Rep of Freedom). The stunning lack of an understanding of the big picture and common good by the GOP is not just sad — but literally tragic.
Kudos to State Rep. Jerry Knirk for a great column in today's Conway Daily Sun which can help us all think about what we're up against (DEC 30). Check it out – by clicking here
Events November 16, 2021 November 16, 2021 Carroll County Democrats
One (Tonight — NOV 16)
Tonight, November 16, in Moultonborough — the Tri Town DEMs will host an event that highlights what is happening with the Free Staters here in NH. Guest speaker is Zandra Rice Hawkins. As DEMs are working to hold on to normalcy, GOP "centrists" like Karen Umberger (Conway) and Mark McConkey (Freedom) are enabling the "No Government Is Good Government" lousiness. Mr. Sununu himself has lamented that his fellow Republicans are falling prey to the conspiracy theories and misinformation coming from the Free Staters and others. Learn more about tonight's event at the Moultonborough Library which starts at 7 PM by clicking: HERE.
Mike Cryans to Greater Ossipee DEMs
November 22 on Zoom — The Greater Ossipee DEMs will welcome Mike Cryans as folks in Carroll County wonder about the power of the Executive Council and the recent weirdness involving councilor Joe Kenney having voted to reject the $27M in federal Covid funds making NH the only state in the country to go without. Thankfully, the Governor and reasonable ones coaxed and dragged Mr. Kenney back to the table where he was strong-armed into accepting $22M. Mr. Cryans is a former executive councilor and will share with us and answer questions. To learn more and to request the Zoom link, click HERE.
Representative Bill Marsh, from the southern floterial House district in our County which includes Brookfield, Effingham, Ossipee, Wakefield, Moultonborough, Sandwich, and Tuftonboro. He has been active in various efforts and discussions since that change. We're looking forward to working with him as he represents us from this side of the aisle in the coming legislative year. Check out a Huffington Post interview with Bill by clicking HERE.
Local elected officials and grassroots activists have been doing great work. On the day for the National Women's March, the Tri-Town Dems had a great visibility demonstration in Center Harbor … a challenging LTE (letter to the editor) from Knute Ogren HERE … Representative Anita Burroughs wonders about the "Free State Project: Follow the Money!" … and Representative Jerry Knirk has been writing a number of great editorials, too, like this THIS important one on Covid and the GOP's bad policy.
Redistricting — And we're all anxious to see what happens with the new redistricting maps! It looks like the Republican majority of the Committee will push through a very gerrymandered district to make it much more difficult for Congressman Pappas to win another term. And our local State representative districts are, in most instances, going to be much different. Ellen Farnum, Town Chair from Tamworth, has been leading a small group of locals to try to give regular feedback and input on the maps. You can see here the proposed maps from the Democratic/Minority and the Republican/Majority Committee members.
The Senate Seat — Chris Sununu is not going to run for the Senate against Maggie Hassan! He will instead seek another term as our Governor – which, of course, we are going to deny him!!! Yes, he's a strong candidate but did you see CCDC Executive Committee Member Leonard Witt's article in the Laconia SUN? The LTE makes a good case for why we can win, with a good candidate, in this next Gubernatorial race! Hassan's campaign office made this statement after Sunono's announcement: "Senator Hassan won her last race by 1,017 votes, and we know that no matter who emerges as the Republican nominee this is going to be a hard-fought race. The Senator has shown that she can work across the aisle to get results for Granite Staters — and that is why she has a record of winning tough races. Our campaign is ready for the challenge ahead."
Can you add 3/three/tres/trois/drei/tin … names to our Carroll County Democrats list? Please?! This newsletter is going out to just over 800 Democrats in our county. There were 16,649 Democratic votes for Biden in the 2020 election. You, or those friends you're going to add to the list, can sign up here.
Facebook — Please remember to "like" and comment on the Carroll County NH Democrats Facebook page. Please encourage your like-minded friends & neighbors to do so as well! Our posts will show on your newsfeed 😉 FACEBOOK
Financial Support — And as always, we appreciate your donations to help elect our Democratic candidates and promote Democratic values – Please click, CONTRIBUTE or mail a check to Carroll County Democrats PO Box 337 Conway, NH 03818. Monthly contributions are very helpful. If you can find your way to making a monthly contribution, it will be very much appreciated.
We're fired up & working hard to return our state to a Democratic majority; to make it clear to the Free Staters that we're going to resist their impact on our communities; to undo the damage of the Trump era; and to return our politics to one of respect for each other.
Thanks for paying attention.
Let me know what you're thinking!
Ed Butler
CC DEMs chairperson
Don't miss out on the opportunity to learn about what the Free Staters are doing to this wonderful state of ours. This is not a new concern, by any means. But it's a concern that is getting more serious with each passing year. The Tri-Town DEMs have invited Zandra Rice Hawkins of Concord to be the featured speaker at their November 16th meeting. They are meeting in-person at Moultonborough Library. Learn More
Consider making a small gift in support of the work of Carroll County DEMs. If everyone makes a small gift every once in a while, we will have all the money we need to be a wonderful support to our 2022 candidates. Click: contribute
When Executive Councilor Joe Kenney voted "NO" on the $27 Million from Washington DC to help with, among other things, vaccinations and other Covid necessities — even GOP Governor Sununu labeled Kenney and his colleagues believers of conspiracy theories. When Kenney bested Cryans in 2020, we did not know that Kenney would be championing ignorance. Join Mike Cryans and the Greater Ossipee DEMs to learn about the Executive Council, why we need a DEM to represent us, and why saying "NO" to those Covid funds have put NH in a pickle. To get your Zoom link for MON, NOV 22 at 7 PM, contact: Knute
And it's never a bad time to be sure that you are registered to vote here in our beautiful state! Here in Carroll County, we have exceedingly helpful folks in our town offices. But you might benefit from taking a look here:
https://sos.nh.gov/elections/information/faqs/how-to-register-to-vote/
Carroll County Caucus — Tonight!
Events May 24, 2021 May 24, 2021 Carroll County Democrats
Join with others from throughout Carroll County for the biennial caucus taking place via Zoom. The leadership of the county is putting forward a list of folks who have the gifts, the passion, and the understanding to move us forward during this upcoming two year cycle. The list:
For Chair — Ed Butler of Hart's Location
For Vice Chair — Theresa Swanick of Effingham
For Secretary — Annie Robbins of Wakefield
For Treasurer — Bill McKay of Tamworth
For At Large Members — Edie DesMarais of Wolfeboro, Leonard Witt of Sandwich, & Erik Corbett (of Conway).
To participate in tonight's caucus at 7 PM, you must request the link by 6 PM by clicking HERE. The Zoom meeting is being hosted by the New Hampshire Democratic Party in Concord.
We are thrilled that we will receive greetings from Senator Maggie Hassan who will be with us at 7 PM — sharp!
Sen. Maggie Hassan to visit Carroll County Caucus
To attend the caucus, you must be a registered DEM living in Carroll County and you must request the link for the caucus by clicking HERE. The New Hampshire Democratic Party leaders in Concord are handling all the Zoom logistics for the county caucus.
We are so pleased that Sen. Maggie Hassan has accepted our invitation to visit with us for a few minutes (assuming there is no legislative floor vote or some other important concern that would pull her away).
The present leadership team of Carroll County DEMs have worked to identify a team of nominees that we think are a great fit for the needs of Carroll County in the next two years. We unanimously endorse the nominees that are listed here:
For Chair: Ed Butler of Hart's Location
For Vice: Theresa Swanick of Effingham
For Sec.: Annie Robbins of Wakefield
For Treas: Bill McKay of Tamworth
At-Large 1: Edie DesMarais of Wolfeboro
At-Large 2: Leonard Witt of Sandwich
At-Large 3: Erik Corbett of Conway
We believe these people have the skills necessary.
We believe it's a HUGE bonus that they are from throughout the whole county.
We believe that this team can move us from "pretty good" to "wicked awesome" as a county.
There are opportunities for nominations to be made from "the floor."
And if you or someone you know would be a good fit — please nominate!!
But … knowing that Zoom meetings make it tough for this kind of thing, the present leadership team wanted to put forward a group of people — and all have said YES (assuming you elect them).
The agenda for the evening will be:
Greetings from Sen. Hassan
Update from State Chair Ray Buckley
The Caucus (electing leaders for the next two year cycle)
Report from out-going chair Knute Ogren
Report from Treasurer Bill McKay about our account balance.
Brief remarks from new leaders
Please join the caucus.
We've come a long way in the last couple of years.
And we are still cooking!!
One more time — Get your CAUCUS ZOOM LINK
Questions? Contact Knute at knute4nh@yahoo.com
Be good.
PS: If you haven't made a contribution to the Carroll County DEMs in a little bit, please consider doing so. If everyone gives a little bit here and and little bit there, we'll have plenty to help our local candidates come 2022! You can do your part by clicking HERE
Training for Treasurers — May 17
Request the Zoom link by emailing knute4nh@yahoo.com. The training will go for about an hour and it will cover pros and cons of having a checking account, what to think about regarding having an account for a regional group, and how to learn from mistakes made in the past. Many thanks to the Carroll County Treasurer, Bill McKay, for his excellent stewardship and care of our funds — and for his willingness to help others learn.
And … don't forget the Carroll County Caucus — May 24 at 7:00 PM. If you haven't yet signed up to participate in the biennial Carroll County Caucus (via Zoom on May 24), you need to sign up — not with Knute — but with the NHDP. We'll be electing leadership for the coming two years. Here's that link: CAUCUS ZOOM REQUEST.
Five Things for May 2021
Events May 6, 2021 May 6, 2021 Carroll County Democrats
May 3: There was a great Zoom event for those who were elected to an officer position in the towns of Carroll County. We'll be doing this again!
May 9: Mother's Day. Buy a card. Make a call. Remember those for whom the day is difficult for any number of reasons.
May 10: A forum and fundraiser for DEMs in NH with special guests Emily Cain of "EMILY's List" and NH State Senator Martha Fuller Clark focussed on *Protecting Reproductive Rights" here in NH and beyond. $25 Ticket
May 24: The biennial County Caucus on Zoom (7 PM) … electing leaders for the upcoming 2 years. We need all DEMs from Carroll County to participate. Zoom Link
May 31: Get ready for Pride Month which begins on June 1!
"Protecting Reproductive Rights" with Emily Cain of EMILY's List. May 10, Zoom
Events April 28, 2021 April 28, 2021 Carroll County Democrats
As a way of staying grounded in some of the most important issues of the day, the "Committee to Elect House Democrats" is hosting an event featuring Emily Cain (of EMILY's List) which will help New Hampshire DEMs think deeply about what's at stake in the fight to protect reproductive rights. The Zoom event — just one hour in length — will be May 10 at 7 PM and has a cost of just $25. Funds raised will be used in a new effort to offer broader support of House candidates in 2022.
The Committee to Elect House Democrats (CEHD) has a new leader and his vision for how DEMs can do better in 2022 is vitally important. Rep. Matt Wilhelm, together with others throughout the state — including our own Anita Burroughs — will be transforming how local candidates receive support and encouragement. We lost in 2020. But we'll win in 2022 because we learned our lesson.
Consider purchasing a $25 ticket to the May 10th event. If you can't attend, but want to participate in the effort to ensure a better 2022 for our House Candidates, you can use the link to make a one-time donation to CEHD. Here's the ticket/donation link: MAY 10 EVENT
Give online to CC DEMs
Or mail a check to:
Carroll County Democrats
Conway, NH 03818

redpajama_set_name: RedPajamaCommonCrawl


If you know the whereabouts of any of these individuals contact CrimeStoppers.
Can you identify any of these suspects? If so, you may qualify for a reward.
Find out more about the GunStoppers initiative.
Do you have information about a crime or on persons who have committed a crime?
What do we mean by anonymous?
If your tip leads to a felony arrest or felony charges you collect a reward!