text:
Man found living in airport for months over COVID fears
By Johanna Garner on January 19, 2021 at 5:00 PM
One man has been found living in Chicago's international airport for three months after COVID-19 left him too scared to fly.
Aditya Singh was arrested over the weekend after he was found living in Chicago's international airport for thee months. Once discovered, the man claimed that he was too scared to go home due to the coronavirus pandemic.
Too scared to fly home
Aditya Singh was arrested on Saturday after airline staff finally asked him to provide his identification. Singh revealed a worker's badge but officials found that it actually belonged to an operations manager who reported it missing months before.
As it turns out, the 36-year-old had been living in the airport for a whole three months. Police revealed that Aditya had arrived at the O'Hare Airport on the 19th of October and had been living off the donations of other travellers.
When questioned, the man cited that he was too scared to fly home due to coronavirus, but authorities later discovered that Singh actually lived in Los Angeles and it is not entirely clear why he was in Chicago.
Cook County Judge Susana Ortiz revealed her surprise at the situation which barred a strange resemblance to The Terminal:
So if I understand you correctly, you're telling me that an unauthorised, non-employee individual was allegedly living within a secure part of the O'Hare airport terminal from 19 October 2020 to 16 January 2021, and was not detected? I want to understand you correctly.
Singh was then ultimately charged with felony criminal trespass to a restricted area of an airport as well as misdemeanour theft and has now been banned from re-entering the airport.
Ortiz revealed that Singh's actions could be considered a threat to the public:
Based upon the need for airports to be absolutely secure so that people feel safe to travel, I do find those alleged actions do make him a danger to the community.
However, the O'Hare Airport has hit back at this claim stating that while the incident was still under investigation, Aditya 'did not pose a security risk to the airport or to the travelling public.'
How can you survive in an airport?
Some may ask just how you can live inside an airport for an extended period, but it's really not that difficult (provided you don't get caught) and has been done quite a few times before.
The most famous of these instances is that of Mehran Nasseri who managed to survive in Terminal One of France's Charles de Gaulle Airport for a total of 18 years.
Nasseri's situation was a bit of a complicated one. After being expelled from Iran in the late '70s, the man was granted refugee status in Belgium where he spent some years before deciding to immigrate to England.
Nasseri had one British parent, which means he qualified for an English passport, but after having his paperwork stolen, he was denied entry to the country and was returned on a flight to France. Nasseri was then arrested in the airport, but it was soon decided that his entry was legal. And, as he also had no 'home country' to be returned to, Nasseri was doomed to remain in the airport.
The ex-Iranian then set himself up in the public space. Accompanied by his luggage, the man spent his days writing in his diary and reading while being fed by airport staff.
During his 18 year stay, both Belgium and France had offered Nasseri new papers and even residency status but he had refused for multiple reasons, mainly that he was determined to go to the UK. In 2006 Nasseri's airport stay ended after he was hospitalized. Since then, he has been assisted by the Red Cross and has been staying in a shelter in Paris.
Back in 2003, Stephen Spielberg bought the right's to Nasseri's story and is said to be the inspiration behind the movieThe Terminal. However, Spielberg failed to acknowledge Nasseri in the credits and ultimately decided not to use his story.
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text:
NLW Archives and Manuscripts
Search Llyfrgell Genedlaethol Cymru = The National Library of Wales
Fonds GB 0210 FOURTS - A. Foulkes-Roberts Manuscripts,
GB 0210 FOURTS
A. Foulkes-Roberts Manuscripts,
[c. 1882]-[1941] / (Creation)
Foulkes-Roberts, Arthur, 1864-1941
Arthur Foulkes-Roberts (1864-1941) of Denbigh was a Fellow of the Society of Antiquaries, Denbigh. He and his brother R.D. Roberts transcribed various parish registers, tombstone inscriptions, church memorials, probate, episcopal and diocesan records, mostly from Denbighshire and Flintshire.
Llyfrgell Genedlaethol Cymru = The National Library of Wales
Donated by Arthur Foulkes-Roberts' son, M.W. Foulkes-Roberts, Ledbury, Herefordshire, 1983.
Notebooks of A. Foulkes-Roberts, [c. 1882]-[1941], containing extracts from parish registers, mainly from Denbighshire and Flintshire; transcripts of tombstone inscriptions and church memorials, copies of probate records from the Dioceses of Bangor and St Asaph, and the Principal Probate Registry; and notes and extracts from marriage licence bonds, clergy subscription books and other St Asaph diocesan records. The copies were made by A. Foulkes-Roberts and his brother R.D. Roberts.
Action: All records donated to the National Library of Wales have been retained..
Accruals are not expected.
Arranged into the following: parish registers, tombstone inscriptions and church memorials; probate records; and episcopal records.
Readers consulting modern papers in the National Library of Wales are required to sign the 'Modern papers - data protection' form.
Usual copyright regulations apply.
English, Welsh.
A hard copy of the catalogue is available in Minor Lists and Summaries 1983, pp. 17-18, at the National Library of Wales.
foulkes-roberts-manuscripts-2.pdf
Transcripts and summaries of other records made by R. D. Roberts with notes by Arthur Foulkes-Roberts are NLW MSS 13,897-13,914, and NLW MSS 14,106-14,119. Further papers of Arthur Foulkes Roberts, including correspondence and papers, pocket diaries, notes and accounts, and local history notes, are at the Denbighshire Record Office.
Title based on content of fonds.
Virtua system control number
vtls003844496
Project identifier
Church records and registers -- Wales -- Denbighshire
Church records and registers -- Wales -- Flintshire.
Wills -- Wales -- Bangor.
Wills -- Wales -- St. Asaph.
Sepulchral monuments -- Wales -- Denbighshire.
Sepulchral monuments -- Wales -- Flintshire.
Dioceses -- Wales -- St. Asaph
St. Asaph (Wales)
Foulkes-Roberts, Arthur, 1864-1941 (Creator)
Roberts, R. D. (Subject)
Description follows ANW guidelines based on ISAD(G) 2nd ed.;AACR2; and LCSH
Compiled by Rhys Jones for the ANW project. The following source was used to compile this description: NLW, Minor Lists and Summaries 1983;
Text: A. Foulkes-Roberts Manuscripts.

redpajama_set_name: RedPajamaCommonCrawl


text:
\section{Introduction}
\label{sec:intro}

Transverse momentum dependent parton distribution functions (TMDPDFs) extend the concept of collinear PDFs,
which describe the longitudinal momentum distribution of quarks and gluons inside protons,
to also reflect their intrinsic transverse motion.
They are important ingredients for describing high-energy scatterings at small transverse momentum,
in particular the Drell-Yan process, an important benchmark observable of the Standard Model
both at the Tevatron~\cite{Affolder:1999jh, Abbott:1999yd, Abazov:2007ac, Abazov:2010kn}
and the LHC~\cite{Aad:2011gj,Chatrchyan:2011wt,Aad:2014xaa,Khachatryan:2015oaa,Aad:2015auj,Khachatryan:2016nbe,Sirunyan:2019bzr,Aad:2019wmn}.
Similarly, they are required for predictions of the Higgs transverse momentum spectrum,
a key observable that is of great interest for the LHC physics program
\cite{Aad:2014lwa,Aad:2014tca,Aad:2016lvc,Aaboud:2017oem,Aaboud:2018xdt,ATLAS:2020wny,Khachatryan:2015rxa,Khachatryan:2015yvw,Khachatryan:2016vnn,Sirunyan:2018kta,Sirunyan:2018sgc}.
TMDPDFs also arise in measurements of semi-inclusive deep-inelastic scattering (SIDIS) \cite{Ashman:1991cj,Derrick:1995xg,Adloff:1996dy,Aaron:2008ad,Airapetian:2012ki,Adolph:2013stb,Aghasyan:2017ctw},
where they are of particular interested because they provide a window into the proton structure~\cite{Boer:2011fh,Accardi:2012qut}.

TMDPDFs measure both the longitudinal momentum fraction $z$ and the transverse momentum ${\vec q}_T$ carried by the struck parton.
They are intrinsically nonperturbative objects that need to be extracted from measurements,
but for perturbative $|{\vec q}_T|$ they can be perturbatively related to collinear PDFs.
Schematically, this matching takes the form
\begin{align} \label{eq:beam_OPE_schematic}
 B_i(z, {\vec q}_T) = \sum_j \int_z^1\!\frac{\mathrm{d} z'}{z'} \, \mathcal{I}_{ij}(z',{\vec q}_T) f_j\Bigl(\frac{z}{z'}\Bigr) \times \bigl[1 + \mathcal{O}(q_T/\Lambda_\mathrm{QCD})\bigr]
\,,\end{align}
where $B_i$ is the so-called TMD beam function for a parton of flavor $i$, the sum runs over all parton flavors $j$, $\mathcal{I}_{ij}$ is the perturbative matching kernel, and $f_j$ is the collinear PDF.
The precise knowledge of $\mathcal{I}_{ij}$ is important for measurements dominated by transverse momenta that are small compared to the hard scale $Q$ of the process but still perturbative, i.e.\ $\Lambda_\mathrm{QCD} \ll |{\vec q}_T| \ll Q$, such as Higgs and Drell-Yan production at the LHC. Precise perturbative predictions for the beam function are also essential to extract the intrinsically nonperturbative corrections, which in global fits is typically achieved through a nonperturbative model on top of \eq{beam_OPE_schematic}, see e.g.~\refscite{Landry:1999an,Landry:2002ix,Konychev:2005iy,DAlesio:2014mrz,Bacchetta:2017gcc,Scimemi:2017etj,Scimemi:2019cmh}.

Since TMDPDFs describe processes at small transverse momentum ${\vec q}_T$, they are intrinsically sensitive to the infrared structure of QCD.
Hence, their perturbative structure is intimately related to the singular structure of QCD amplitudes.
This property is employed in the $q_T$ subtraction scheme proposed in \refcite{Catani:2007vq}
to achieve the cancellation of infrared divergences in next-to-next-leading order (NNLO) calculations of color-singlet cross sections.
Recently, extensions of this method to next-to-next-to-next-to-leading order (N$^3$LO) were discussed in \refscite{Cieri:2018oms,Billis:2019vxg}, which however did not include the required three-loop ingredient.

TMDPDFs are composed of the TMD beam function $B_i(z,{\vec q}_T)$ and the TMD soft function $S({\vec q}_T)$.
The soft function has been known at three loops since quite some time~\cite{Echevarria:2015byo,Li:2016ctv,Luebbert:2016itl},
and the quark beam function has been calculated at this accuracy recently~\cite{Catani:2012qa,Gehrmann:2012ze,Gehrmann:2014yya,Echevarria:2016scs,Luo:2019hmp,Luo:2019szz},
while the gluon beam function so far is only known at two loops~\cite{Catani:2011kr,Gehrmann:2014yya,Echevarria:2016scs,Luo:2019bmw}.
In this paper, we fill this gap by calculating the full matching coefficient for the gluon beam function at N$^3$LO.
We also calculate the full quark beam function at N$^3$LO, where we find disagreement with the recent calculation of the corresponding result in \refcite{Luo:2019szz} in the $d_{abc} d^{abc}$ color structure.
These results make it possible to fully apply the ${\vec q}_T$ subtraction at N$^3$LO accuracy,
paving the way for fully-differential cross sections of color-singlet processes at this order.
Our results are also the last missing ingredient for TMD resummation at N$^3$LL$^\prime$ accuracy.
They also arise in ${\vec q}_T$-dependent event shapes at hadron colliders such as the Transverse Energy-Energy Correlator (TEEC)~\cite{Gao:2019ojf}, and for the azimuthal angle in vector boson $+j$ production in the back-to-back limit~\cite{Chien:2019gyf, Chien:2020hzh}.

We perform the calculation of the TMDPDF at N$^3$LO by using the framework of the collinear expansion of cross sections presented in~\cite{Ebert:2020lxs}.
This framework allows us to efficiently compute universal building blocks of perturbative QFT in kinematic limits leveraging on modern technology developed for the computation of multiloop scattering cross sections.
In particular, we expand the diagrams for the Drell-Yan and gluon fusion Higgs boson production cross section at N$^3$LO in the collinear limit.
We make use of the framework of reverse unitarity~\cite{Anastasiou2003,Anastasiou:2002qz,Anastasiou:2003yy,Anastasiou2005,Anastasiou2004a} to enforce measurement and on-shellness constraints on the final states as well as integration-by-part (IBP) identities~\cite{Chetyrkin:1981qh,Tkachov:1981wb} and the method of differential equations~\cite{Kotikov:1990kg,Kotikov:1991hm,Kotikov:1991pm,Henn:2013pwa,Gehrmann:1999as} to obtain the cross sections differential in the rapidity and transverse momentum of the colorless final states in the collinear limit.
Following \refcite{Ebert:2020lxs}, we exploit this limit of the differential cross sections to extract the bare matching kernels of the quark and gluon ${\vec q}_T$ beam functions.

This paper is structured as follows. In \sec{factorization}, we briefly review TMD factorization.
In \sec{coll_exp}, we discuss how the beam function can be calculated from the collinear limit of a color-singlet cross section using the method collinear expansions.
In \sec{results}, we present our results, before concluding in \sec{conclusion}.
Our results are also available in electronic form in the ancillary files of this submission.

\section{Review of \texorpdfstring{\boldmath $q_T$}{qT} factorization}
\label{sec:factorization}

We study the production of a color-singlet state $h$
and an additional hadronic state $X$ in a proton-proton scattering process,
\begin{align} \label{eq:process_hadr}
 P(P_1) + P(P_2) \quad\to\quad h(-p_h) + X(-k)
\,,\end{align}
where we align the incoming protons along the directions
\begin{align} \label{eq:nnb}
 n^\mu = (1,0,0,1) \,,\qquad {\bar n}^\mu = (1,0,0,-1)
\end{align}
and denote their momenta as $P_1$ and $P_2$, with the center of mass energy being $S=(P_1+P_2)^2$.
We are interested in measuring the cross section differential in $p_h^\mu$,
expressed through the invariant mass $Q^2 = p_h^2$, rapidity $Y$, and transverse momentum ${\vec q}_T$.

The factorization of the cross section in the limit $q_T \ll Q$ was first established by Collins, Soper, and
Sterman (CSS)~\cite{Collins:1981uk,Collins:1981va,Collins:1984kg},
and was further elaborated on in \refscite{Catani:2000vq,deFlorian:2001zd,Catani:2010pd,Collins:1350496}.
The factorization was also shown using Soft-Collinear Effective Theory (SCET)
\cite{Bauer:2000ew, Bauer:2000yr, Bauer:2001ct, Bauer:2001yt}
by several groups \cite{Becher:2010tm,Becher:2011xn,Becher:2012yn,GarciaEchevarria:2011rb,Echevarria:2012js, Echevarria:2014rua,Chiu:2012ir,Li:2016axz}.
The factorized cross section is typically expressed in Fourier space in two equivalent forms,
\begin{align} \label{eq:TMD_factorization}
 \frac{\mathrm{d}\sigma}{\mathrm{d} Q^2 \mathrm{d} Y \mathrm{d}^2 {\vec q}_T} &
 = \sigma_0 \sum_{a,b} H_{ab}(Q^2,\mu) \int\!\frac{\mathrm{d}^2{\vec b}_T}{(2\pi)^2} e^{\mathrm{i}\,{\vec q}_T \cdot {\vec b}_T}
   \,\tilde B_a\Bigl(x_1^B, b_T, \mu, \frac{\nu}{\omega_a}\Bigr)
   \,\tilde B_b\Bigl(x_2^B, b_T, \mu, \frac{\nu}{\omega_b}\Bigr)
   \, \tilde S(b_T, \mu, \nu)
\nonumber\\&
 = \sigma_0 \sum_{a,b} H_{ab}(Q^2,\mu) \int\!\frac{\mathrm{d}^2{\vec b}_T}{(2\pi)^2} e^{\mathrm{i}\,{\vec q}_T \cdot {\vec b}_T}
   \,\tilde f_a(x_1^B, b_T, \mu, \zeta_a) \, \tilde f_b(x_2^B, b_T, \mu, \zeta_b)
\,.\end{align}
For processes inclusive in $h$, \eq{TMD_factorization} holds up to corrections in $\mathcal{O}(q_T^2/Q^2)$. Power corrections of $\mathcal{O}(q_T^2/Q^2)$ have been firstly calculated at fixed order in perturbation theory in \refcite{Ebert:2018gsn}, while the study of their all order structure has been initiated using SCET operator formalism~\cite{Kolodrubetz:2016uim,Feige:2017zci,Moult:2017rpl,Chang:2017atu,Chang:NLP} and their nonperturbative structure has been explored in \refscite{Balitsky:2017gis,Balitsky:2017flc}.
\Eq{TMD_factorization} receives enhanced $\mathcal{O}(q_T/Q)$ corrections when applying fiducial cuts to $h$ \cite{Ebert:2019zkb} that can be uniquely included in the factorization for Higgs and Drell-Yan production~\cite{Ebert:fiducial}, and also receives linear corrections when radiation from massive final states is considered \cite{Buonocore:2019puv}.

In \eq{TMD_factorization}, we sum over all parton flavors $a$ and $b$ mediating
the underlying partonic process $ab \to h$. The corresponding partonic
Born cross section is denoted by $\sigma_0$, and the hard function $H_{ab} = 1 + \mathcal{O}(\alpha_s)$
encodes virtual corrections to the Born process.
For Drell-Yan and gluon fusion Higgs production in the $m_t\to\infty$ limit, the N$^3$LO hard function can be found in \refcite{Gehrmann:2010ue}, and for $b \bar{b} \to H$ in \refscite{Gehrmann:2014vha,Ebert:2017uel}.
The $\tilde B_i(x,b_T,\mu,\nu/\omega)$ encode the probability to find a parton of flavor $i$
with longitudinal momentum fraction $x$ and impact parameter ${\vec b}_T$, which is Fourier-conjugate to ${\vec q}_T$.
The soft function $\tilde S$ encodes the effect of soft radiation from either proton.
In the second line of \eq{TMD_factorization}, these functions are combined into the TMDPDF
\begin{equation}\label{eq:TMDPDFdef}
 \tilde f_i(x, b_T, \mu, \zeta) = \tilde B_i\Bigl(x, b_T, \mu, \frac{\nu}{\sqrt\zeta}\Bigr) \sqrt{S(b_T, \mu, \nu)}
\,,\end{equation}
which is indepdent of the rapidity scale $\nu$ discussed below.
Computationally, it is natural to separately consider
the calculation of the beam and soft functions appearing in \eq{TMD_factorization},
which can easily be combined into the TMDPDF if desired.

A characteristic feature of $q_T$ factorization is the appearance of so-called
rapidity divergences~\cite{Collins:1981uk,Collins:2008ht,Becher:2010tm,GarciaEchevarria:2011rb,Chiu:2011qc,Chiu:2012ir,Rothstein:2016bsq},
which require an explicit rapidity regulator. Similar to the emergence of the
renormalization scale $\mu$ from ultraviolet (UV) regularization, this induces a rapidity scale,
which we generically as $\nu$. The rapidity divergences track the energy of the
struck partons, encoded in the parameters
\begin{align}
 \omega_a = x_a \, {\bar n} \cdot P_a = Q e^{+Y}
\,,\quad
 \omega_b = x_b \, n \cdot P_b = Q e^{-Y}
\,,\qquad
 \zeta_{a,b} \propto \omega_{a,b}^2\quad\mathrm{s.t.}\quad\mathrm\zeta_a \zeta_b = Q^4
\,.\end{align}
There is a variety of rapidity regulators, giving rise to several formulations
of the individual ingredients in \eq{TMD_factorization}. However, all approaches
yield the same fixed-order results for the physical cross section in \eq{TMD_factorization}.
Thus, we are free to choose the regulator most convenient for our calculation,
and we will employ the exponential regulator of \refcite{Li:2016axz}.
Explicit definitions of the beam and soft functions in terms of gauge-invariant
matrix elements formulated in SCET can be found in \refcite{Li:2016axz}
(see also \refscite{Luo:2019hmp,Luo:2019bmw}), but are not required in our approach.

In this work, we focus on TMD factorization in the perturbative regime $b_T^{-1} \sim q_T \gg \Lambda_\mathrm{QCD}$,
in which the TMD beam function and TMDPDF can be matched onto PDFs as \cite{Collins:1984kg}
\begin{align} \label{eq:beam_OPE}
 \tilde B_i\Bigl(z, b_T, \mu, \frac{\nu}{\omega}\Bigr) &
 = \sum_j \int_z^1\!\frac{\mathrm{d} z'}{z'} \, \tilde \mathcal{I}_{ij}\Bigl(z', b_T, \mu, \frac{\nu}{\omega}\Bigr)
   f_j\Bigl(\frac{z}{z'},\mu\Bigr) \times \bigl[1 + \mathcal{O}(b_T \Lambda_\mathrm{QCD})\bigr]
\,,\nonumber\\
 \tilde f_i(z, b_T, \mu, \zeta) &
 = \sum_j \int_z^1\!\frac{\mathrm{d} z'}{z'} \, \tilde\mathcal{I}^{\rm TMD}_{ij}(z', b_T, \mu, \zeta)
   f_j\Bigl(\frac{z}{z'},\mu\Bigr) \times \bigl[1 + \mathcal{O}(b_T \Lambda_\mathrm{QCD})\bigr]
\,.\end{align}
The matching kernels $\tilde\mathcal{I}_{ij}$ and $\tilde\mathcal{I}^{\rm TMD}_{ij}$ are the objects of interest of this paper.

\section{Beam functions from the collinear limit of cross sections}
\label{sec:coll_exp}

We consider the contribution to \eq{process_hadr} from the partonic process
\begin{align} \label{eq:process_part}
 i(p_1) + j(p_2) \quad\to\quad h(-p_h) + X_n(-p_3, \dots, -p_{n+2})
\,.\end{align}
The incoming partons carry momentum $p_1$ and $p_2$ and flavor $i$ and $j$, respectively, while we denote with $X_n$ the hadronic final state with total momentum $k$, consisting of $n$ partons with momenta $\{-p_3, \dots, -p_{n+2}\}$, such that $k = \sum_{i\ge3} p_i$. Note that at tree level we have $n=0$.

The final-state momenta are parameterized in terms of
\begin{align} \label{eq:vardef}
 Q^2 = p_h^2
 \,, \quad
 Y = \frac12 \ln\frac{{\bar n} \cdot p_h}{n \cdot p_h}
 \,, \quad
 {w_1} = -\frac{\bar n\cdot k}{\bar n \cdot p_1}
 \,,\quad
 {w_2} = -\frac{ n\cdot k}{ n \cdot p_2}
 \,,\quad
 x = \frac{k^2}{(\bar n\cdot k)(n\cdot k)}
\,,\end{align}
where $Y$ is the rapidity of the color-singlet state $h$ and $Q^2$ its invariant mass.

The partonic cross section differential in these variables is defined as
\begin{align} \label{eq:sigma_part}
  \frac{\mathrm{d} \eta_{ij}}{ \mathrm{d} Q^2  \mathrm{d} {w_1} \mathrm{d} {w_2} \mathrm{d}  x}  &
 = \frac{1}{\sigma_0} \frac{\mathcal{N}_{ij}}{2 S} \sum_{X_n}\int  \frac{\mathrm{d}\Phi_{h+n} }{ \mathrm{d} {w_1} \mathrm{d} {w_2} \mathrm{d}  x}\, |\mathcal{M}_{ij\to h+X_n}|^2
\,.\end{align}
Here $\mathrm{d}\Phi_{h+n}$ represents the differential phase space measure for the $h+X_n$ state,
$|\mathcal{M}_{ij\to h+X_n}|^2$ is the squared matrix element for the partonic process in \eq{process_part},
summed over the colors and helicities of the particles, with $\mathcal{N}_{ij}$ containing the helicity and color average of the incoming particles, and we normalize the expression by $\sigma_0$, the partonic Born cross section. The interested reader can find explicit expressions for $\mathcal{N}_{ij}$ and $\mathrm{d}\Phi_{h+n}$ in \refcite{Ebert:2020lxs}.

In \refcite{Ebert:2020lxs}, we showed that the matching coefficient in \eq{beam_OPE} is obtained by taking the limit of \eq{sigma_part} where all real and loop momenta are treated as being collinear to $n$-direction, which is referred as the \emph{strict} $n$-collinear limit, and we refer to \refcite{Ebert:2020lxs} for details on its calculation:
\begin{align} \label{eq:Iij_naive}
 \mathcal{I}_{ij}^{\rm naive}(z,q_T)
 = \int_0^1 \mathrm{d} x \int_0^\infty \mathrm{d} {w_1}\mathrm{d} {w_2} \,&
   \delta[z - (1-{w_1})] \, \delta\Big[q_T^2 - \frac{{w_1}{w_2}}{1-{w_1}} (1-x) Q^2\Bigr]
   \nonumber\\&\times\,
   \lim\limits_{\mathrm{strict}~n-\mathrm{coll.}} \frac{\mathrm{d}\eta_{ij}}{\mathrm{d} Q^2  \mathrm{d}{w_1} \mathrm{d}{w_2} \mathrm{d} x}
\,.\end{align}
Solving the $\delta$ functions fixes ${w_1}$ and ${w_2}$ as
\begin{align} \label{eq:vars_LP}
 {w_1} = 1-z \,,\quad
 {w_2} = \frac{q_T^2}{Q^2} \frac{z}{(1-x)(1-z)}
\,.\end{align}
The superscript $^{\rm naive}$ in \eq{Iij_naive} indicates that further steps are required to obtain the desired matching kernel. First, we note that the integral in \eq{Iij_naive} contains the aforementioned rapidity divergences, namely divergences as $x\to1$ or $z\to1$ that are not regulated by dimensional regularization. We regulate these using the exponential regulator of \refcite{Li:2016axz}, which in fact is the only regulator in the literature compatible with our approach.
Inserting the regulator factor $\exp(2 \tau e^{-\gamma_E} k^0)$ expressed in the above variables, we obtain the regulated kernel as \cite{Ebert:2020lxs}
\begin{align} \label{eq:Iij_bare}
 \mathcal{I}_{ij}(z,q_T,\epsilon,\tau/\omega) = \lim_{\substack{\tau\to0\\\epsilon\to0}} \int_0^1\mathrm{d} x &\,\frac{z}{Q^2 (1-x)(1-z)}
 \exp\left[ - \tau e^{-\gamma_E} \frac{q_T^2}{\omega} \frac{z}{(1-x)(1-z)}\right]
 \nonumber\\&\times
 \lim\limits_{\mathrm{strict}~n-\mathrm{coll.}} \frac{\mathrm{d}\eta_{ij}}{\mathrm{d} Q^2  \mathrm{d} {w_1} \mathrm{d} {w_2} \mathrm{d} x}\biggl|_{\eqref{eq:vars_LP}}
\,.\end{align}
Here, $\omega = Q e^Y$ is the so-called label momentum. The exponential factor in \eq{Iij_bare} regulates divergences as $x,z\to1$, with $\tau$ being the rapidity regulator. UV and IR divergences are regulated by working in $d=4-2\epsilon$ dimensions, with the limit $\epsilon\to0$ being taken after the limit $\tau\to0$, as indicated. It is convenient to expand the exponential factor in \eq{Iij_bare} in terms of distributions before carrying out the integral~\cite{Luo:2019hmp}, and we provide more details on this in \app{rapidity_regulator}.

It is common to express TMD beam functions in Fourier space, where convolutions in ${\vec q}_T$ are replaced by simple products, which in particular greatly simplifies the resummation of large logarithms~\cite{Ebert:2016gcn}.
Denoting the Fourier-transform matching kernel as $\tilde\mathcal{I}_{ij}$, we obtain the renormalized kernel as
\begin{equation} \label{eq:Iij_ren}
 \tilde \mathcal{I}_{ij}(z,b_T,\mu,\nu/\omega)
 = \sum_{k} \int_z^1\!\frac{\mathrm{d} z'}{z'} \, \Gamma_{jk}\Bigl(\frac{z}{z'}, \epsilon\Bigr) \,
   \tilde Z_B^i(\epsilon,\mu,\nu/\omega) \, \hat Z_{\alpha_s}(\mu,\epsilon) \,
   \frac{\tilde \mathcal{I}_{i k}(z',b_T,\epsilon,\tau)}{\tilde S(b_T,\epsilon,\tau)}
.\end{equation}
Here, following \refcite{Li:2016ctv} we identify $\nu \equiv 1/\tau$ as the rapidity renormalization scale~\cite{Chiu:2012ir}.
The so-called zero-bin subtraction~\cite{Manohar:2006nz} to subtract overlap of the beam function with the soft function is implemented by dividing by the soft function $\tilde S$~\cite{Luo:2019hmp}.
In \eq{Iij_ren}, the counterterm $\hat Z_{\alpha_s}$ implements the renormalization of the bare coupling constant $\alpha_s^b$ in the $\overline{\mathrm{MS}}$ scheme as stated in \eq{asb}.
Infrared divergences are canceled through the convolution with the PDF counterterm $\Gamma_{jk}$, which is given in \eq{Gamma}.
The remaining poles in $\epsilon$ are of UV nature in SCET and are thus canceled by an additional UV counter term in the effective theory, which is the beam function counter term $\tilde Z_B$.

Since the bare soft function is not given in the literature, we have directly calculated it from the soft limit of \eq{sigma_part} similar to \eq{Iij_bare}.
\begin{align} \label{eq:S_bare}
 S (q_T,\epsilon,\tau)
 = \lim_{\substack{\tau\to0\\\epsilon\to0}}&
   \int_0^1\mathrm{d} x \int_0^\infty \, \mathrm{d} w_1 \mathrm{d} w_2 \,
   \delta\bigl[q_T^2 - {w_1}{w_2} (1-x) Q^2\bigr]
\nonumber\\&\times
   \exp\bigl[-2 Q \tau e^{-\gamma_E} ({w_1} + {w_2})\bigr]
   \lim\limits_{\text{strict soft}} \frac{\mathrm{d}\eta_{ij}}{\mathrm{d} Q^2  \mathrm{d} {w_1} \mathrm{d} {w_2} \mathrm{d} x}
\,.\end{align}
In the strict soft limit, both ${w_1}$ and ${w_2}$ are treated as small quantities, such the measurement $\delta$ function and the exponential regulator in \eq{S_bare} are simpler than in \eq{Iij_naive}.
The Fourier transform of \eq{S_bare} yields the bare soft function $\tilde S(b_T,\epsilon,\tau)$ required in \eq{Iij_ren}. We have also verified that the renormalized soft function reproduces the N$^3$LO result of \refcite{Li:2016ctv}.
Since the bare soft function in the exponential regulator is only given at NLO in the literature~\cite{Li:2016axz}, we provide the bare soft function in electronic format in the ancillary files.

The strict soft limit of the general differential partonic coefficient function is obtained by expanding the strict collinear limit in $w_1$ and maintaining only the first term of the generalised power series.
At $n^{th}$ order in perturbation theory  the strict soft limit of the partonic coefficient function takes the form
\begin{equation} \label{eq:soft_limit}
\lim\limits_{\text{strict soft}} \frac{\mathrm{d}\eta_{ij}^{(n)}}{\mathrm{d} Q^2  \mathrm{d} {w_1} \mathrm{d} {w_2} \mathrm{d} x}= \omega_1^{-1-n\epsilon} \omega_2^{-1-n\epsilon} \eta^{(n)}_{\text{strict soft}} (x,\epsilon),
\end{equation}
where $\eta^{(n)}_{\text{strict soft}} (x,\epsilon)$ is independent of $w_1$ and $w_2$.
Note that \eq{soft_limit} is related to the bare fully-differential soft function which measures the total soft radiation in a process.
This limit is also easily related to the bare threshold soft function~\cite{Li:2014afw} via
\begin{equation}
S_{\text{thr}}^{(n)}(z,\epsilon)=\int_0^\infty \mathrm{d} w_1 \, \mathrm{d} w_2 \int_0^1 \mathrm{d} x \, \delta(1-z-w_1-w_2 ) \eta^{(n)}_{\text{strict soft}} (x,\epsilon)\,,
\end{equation}
where $z$ is the threshold parameter.
We have used this relation as an additional check on our soft limit.

\section{Results}
\label{sec:results}

Here, we present our results for the matching kernels of the TMD beam functions at N$^3$LO.
Our calculation leverages on the collinear expansion of the cross sections for off-shell photon production (Drell-Yan) and Higgs production in gluon fusion in proton-proton collisions.
The computation of the Higgs boson production cross section is performed in the heavy top quark effective theory where the gluons are directly coupled to the Higgs boson via an effective operator generated by integrating out the top quark field from the SM Lagrangian~\cite{Inami1983,Shifman1978,Spiridonov:1988md,Wilczek1977,Chetyrkin:1997un,Schroder:2005hy,Chetyrkin:2005ia,Kramer:1996iq,Kniehl:2006bg}.
The matrix elements for this computation can be categorized by the number of final state partons in addition to the color singlet final state. The relevant matrix elements for the calculation of the N$^3$LO differential cross sections in the collinear limit involve one (RVV), two (RRV) and three (RRR) final state partons.

The results for the partonic cross sections involving matrix elements with exactly one parton in the final state are available in full kinematics from refs.~\cite{Duhr:2020seh,Dulat:2014mda,Dulat:2017brz,Dulat:2017prg} which build on previous work done in refs.~\cite{Anastasiou:2013mca,Duhr:2014nda,Duhr:2013msa}.
Therefore, in order to obtain the RVV contributions in the strict collinear limit, we can straightforwardly expand the results in full kinematics and extract the required components.

To compute the collinear limit of the partonic cross sections with more than one final state parton, the necessary Feynman diagrams are obtained using QGRAF~\cite{Nogueira_1993}. We carry out the spinor and color algebra using an in-house code, and perform the strict collinear expansion of these matrix elements following the procedure outlined in ref.~\cite{Ebert:2020lxs}.
In order to integrate over loop and phase space momenta with measurement and on-shell constraints, we make use of the framework of reverse unitarity~\cite{Anastasiou2003,Anastasiou:2002qz,Anastasiou:2003yy,Anastasiou2005,Anastasiou2004a}.

We re-express our expanded cross section in terms of master integrals (MI) via integration-by-parts (IBP) identities~\cite{Chetyrkin:1981qh,Tkachov:1981wb}. We obtain a basis of 492 MI, expressed in terms of the variables in \eq{vardef} as well as the dimensional regularization parameter $\epsilon$, of which 172 MI are required to describe the RRV contributions, while 320 are needed for the RRR ones.
In order to compute the collinear master integrals we employ the method of differential equations~\cite{Kotikov:1990kg,Kotikov:1991hm,Kotikov:1991pm,Henn:2013pwa,Gehrmann:1999as}.
We fix the boundary conditions for the differential equations by further expanding the collinear master integrals in the soft limit and integrating over the phase space, such that the result of this procedure can then be easily matched to the soft integrals calculated in \refscite{Anastasiou:2013srw,Anastasiou:2014lda,Anastasiou:2014vaa,Anastasiou:2015yha,Duhr:2019kwi}.

Completing these steps we obtain the bare differential partonic cross section expanded in the strict collinear limit of \eq{sigma_part}.
We note that the ingredients computed so far are the same as those neeeded for the calculation of the N$^3$LO $N-$jettiness beam functions of \refcite{Ebert:2020unb}.
Next, we obtain the bare matching kernel via \eq{Iij_bare} and subsequently perform the Fourier transform over ${\vec q}_T$ using \eq{FT_qT}.
Both the calculation of the differential partonic cross section as well as the extration of the ${\vec q}_T$-dependent matching kernels will be elaborated in ref.~\cite{Ebert:ThingsToCome}.
Finally, the renormalized matching kernel is obtained using \eq{Iij_ren},
where the beam function counter term $\tilde Z_B^i$ was predicted from the renormalization group equations (RGEs) of the beam function as shown in \app{counter_term}.
The TMDPDF can then be straightforwardly obtained by combining the beam function with the soft function as in \eq{TMDPDFdef}.

We expand the matching kernels $\tilde\mathcal{I}_{ij}$ of the beam function and the matching kernels $\tilde\mathcal{I}^{\rm TMD}_{ij}$ of the TMDPDF obtained in this way in powers of $\alpha_s/\pi$,
\begin{align}
 \tilde\mathcal{I}_{ij}(z,b_T,\mu,\nu/\omega) &
 = \sum_{\ell=0}^\infty \Bigl(\frac{\alpha_s}{\pi}\Bigr)^\ell \tilde\mathcal{I}_{ij}^{(\ell)}(z,b_T,\mu,\nu/\omega)
\,,\nonumber\\
 \tilde\mathcal{I}^{\rm TMD}_{ij} (z,b_T,\mu,\zeta) &
 = \sum_{\ell=0}^\infty \Bigl(\frac{\alpha_s}{\pi}\Bigr)^\ell \tilde\mathcal{I}^{\mathrm{TMD}\,(\ell)}_{ij}(z,b_T,\mu,\zeta)
\,,\end{align}
where the coefficients $\tilde\mathcal{I}_{ij}^{(\ell)}$ and $\tilde\mathcal{I}^{\mathrm{TMD}~(\ell)}_{ij}$ can be written as a polynomial in logarithms of the appearing scales with $z$-dependent coefficient functions,
\begin{align}\label{eq:logdef}
 \tilde\mathcal{I}_{ij}^{(\ell)}(z,b_T,\mu,\nu/\omega) &= \sum_{m,n=0}^\ell \tilde\mathcal{I}_{ij}^{(\ell,m,n)}(z) L_b^n L_\omega^m
\,,\\\nonumber
 \tilde\mathcal{I}^{\mathrm{TMD}\,(\ell)}_{ij}(z,b_T,\mu,\zeta) &= \sum_{n=0}^{2\ell} \sum_{m=0}^{\ell} \tilde\mathcal{I}^{\mathrm{TMD}~(\ell,m,n)}_{ij}(z) L_b^n L_\zeta^m
\,.\end{align}
The logarithms in \eq{logdef} are defined as
\begin{align}
 L_b = \ln\frac{b_T^2 \mu^2}{4 e^{-2\gamma_E}}
 \,,\qquad L_\omega = \ln\frac{\nu}{\omega}
 \,,\qquad L_\zeta = \ln\frac{\mu^2}{\zeta}
\,,\end{align}
where $\gamma_E$ is the Euler-Mascheroni constant, and we remind the reader that $\zeta=\omega^2$ is the energy of the struck parton.
The logarithmic terms with $m > 0$ or $n > 0$ in \eq{logdef} fully describe the scale dependence of both the TMDPDF as well as of the beam function. Therefore, their structure is completely determined by the beam function RGEs (see \app{RGEs}) in terms of its anomalous dimensions and lower-order ingredients.
The nonlogarithmic beam function boundary term at N$^3$LO
\begin{equation}
 \tilde I_{ij}^{(3)}(z) \equiv \tilde\mathcal{I}_{ij}^{(3,0,0)}(z)
\,,\end{equation}
is the genuinely new result calculated by us in this work.
Remarkably, it can be expressed entirely in terms of standard plus distributions and harmonic polylogarithms~\cite{Remiddi:1999ew} of argument $z$ and transcendental weight less or equal to five.
To allow for an easy numeric implementation, we also provide a generalized power series expansion of our results around $z=0$ and $z=1$ with up to 50 terms in each expansion.
Both expansions formally converge in the unit interval, but, clearly, the convergence of the series improves as the expansion parameter gets smaller.
In the ancillary files of the arXiv submission of this article we provide both power series as well as the analytic solution for all matching kernels.

We performed several checks on our results. Firstly, we verified that the UV and IR subtraction as given in \eq{Iij_ren} correctly removes all poles in $\epsilon$. Our NLO and NNLO results for the renormalized beam function are validated against \refcite{Luebbert:2016itl}, and the bare results through $\mathcal{O}(\epsilon^4)$ at NLO and through $\mathcal{O}(\epsilon^2)$ are verified against \refscite{Luo:2019hmp,Luo:2019bmw}.
Given that the logarithmic terms in \eq{logdef} are dictaded by the beam function RGE, we verify that all logarithmic terms of our result are correct by comparing them against those predicted in \refcite{Billis:2019vxg} by solving the beam function RGE.
We also verified the eikonal limit
\begin{align} \label{eq:eikonal_limit}
 \lim_{z\to1} \tilde I_{ij}^{(3)}(z) &
 = \frac{\gamma_2^r}{64} \, \delta_{ij} \, \mathcal{L}_0(1-z)
\,,\end{align}
which was derived in \refcite{Billis:2019vxg} from consistency with joint $q_T$ and soft threshold resummation relations~\cite{Li:2016axz,Lustermans:2016nvk}, and also conjectured in \refcite{Echevarria:2016scs}.
In \eq{eikonal_limit}, $\gamma_2^r$ is the three-loop coefficient of the so-called rapidity anomalous dimension~\cite{Chiu:2012ir}, as given in Eq.~(16) of \refcite{Li:2016ctv} (see also \refcite{Vladimirov:2016dll}), where the appropriate color structure is implicit.
The rapidity anomalous dimensions is also closely related to the Collins-Soper kernel of \refscite{Collins:1981uk,Collins:1981va}.
For the quark beam function, we also compared with the results recently obtained in \refcite{Luo:2019szz}. We find discrepancies for terms proportional to the color structure $d^{abc}d_{abc}$ entering in all quark-to-quark kernels. After private communication, the authors of~\refcite{Luo:2019szz} identified and resolved a minor mistake in their calculation, after which they find agreement with our result.
Furthermore, another check of our results comes from the fact that the first four terms in the soft expansion of the Higgs cross section correctly match the collinear limit of the threshold expansion of the partonic cross section obtained in ~\refcite{Dulat:2017prg,Dulat:2018bfe}.
We also note that inclusive cross section for Drell-Yan as well as for Higgs production at N$^3$LO was calculated in \refscite{Anastasiou:2015ema,Duhr:2020seh,Mistlberger:2018etf,Anastasiou:2014lda,Anastasiou:2014vaa}.
Using the collinear partonic coefficient functions of our calculation after integration over phase space, we also correctly reproduce the leading threshold expansion contribution of all partonic initial states that contribute to the collinear limit of the partonic cross sections.

\begin{figure*}
 \centering
 \includegraphics[width=0.49\textwidth]{plots/I3_quark.pdf}
 \hfill
 \includegraphics[width=0.49\textwidth]{plots/I3_gluon.pdf}
 \caption{The N$^3$LO beam function boundary term $\tilde I^{(3)}_{ij}(z)$ as a function of $z$ in all channels contributing to the quark beam function (left) and the gluon beam function (right). The different channels are rescaled as indicated in the figures.}
 \label{fig:I3}
\end{figure*}

Let us numerically illustrate our results. In \fig{I3} we plot the beam function boundary terms $\tilde I_{ij}(z)$ for the quark (left) and gluon (right) beam functions as a function of $z$. Note that in this plot we set $\delta(1-z) \to 0$ and replaced the distribution $\mathcal{L}_0(1-z) \to (1-z)^{-1}$.
For illustration purposes we rescaled the different channel as indicated, given that they give rise to very different shapes and magnitudes.

Next, we study the impact of our calculation on the beam function and TMDPDF themselves.
We use the \texttt{MMHT2014nnlo68cl} PDF of \refcite{Harland-Lang:2014zoa}, using $\alpha_s(m_Z)=0.118$ and the evaluation of \eq{beam_OPE} is obtained through an implementation of our results in \texttt{SCETlib}~\cite{scetlib}.

\begin{figure*}
 \centering
 \includegraphics[width=0.49\textwidth]{plots/TMDPDF_convergence_u.pdf}
 \hfill
 \includegraphics[width=0.49\textwidth]{plots/TMDPDF_convergence_g.pdf}
 \caption{The $u$-quark TMDPDF (left) and the gluon TMDPDF (right) as a function of $z$ for fixed $b_T = (10~\,\mathrm{GeV})^{-1}$ and $\mu=\omega=100~\,\mathrm{GeV}$. We show the result at LO (which corresponds to the PDF), NLO, NNLO and N$^3$LO.}
 \label{fig:TMDPDF_convergence}
\end{figure*}

In \fig{TMDPDF_convergence}, we show the $u$-quark TMDPDF (left) and the gluon TMDPDF (right) at different orders in the coupling constant%
\footnote{Note that while varying the perturbative order of the matching kernel we keep the \texttt{MMHT2014nnlo68cl} PDF fixed. It is also interesting to study the simultaneously variation of both the order of the matching kernel as well as that of the PDF on which the beam function gets matched onto. However, an extraction of PDFs at N$^3$LO is currently not available and while there are methods to the study the uncertainty due to missing higher order PDFs \cite{Anastasiou:2016cez,Forte:2013mda}, this is clearly independent of the calculation of the matching kernel.}
as a function of $z$.
We fix the impact parameter $b_T = 10~\,\mathrm{GeV}^{-1}$, parton energy $\omega = 100~\,\mathrm{GeV}$ and renormalization scale $\mu = 100~\,\mathrm{GeV}$.
Since the LO result for the beam function corresponds to the PDF itself, \fig{TMDPDF_convergence} can be used to appreciate the difference in shape of the beam function compared to the PDF. With the inclusion of the N$^3$LO result obtain in this work, both the quark and the gluon TMDPDFs nicely show convergence over a large range of values for $z$.

\begin{figure*}
 \centering
 \includegraphics[width=0.49\textwidth]{plots/ratio_LO_u.pdf}
 \hfill
 \includegraphics[width=0.49\textwidth]{plots/ratio_LO_g.pdf}
 \caption{The relative difference of $u$-quark beam function (left) and the gluon beam function (right) to the corresponding PDF, as a function. We fix $b_T = (10~\,\mathrm{GeV})^{-1}$ and $\omega=100~\,\mathrm{GeV}$ and choose the canonical scales $\mu b_T = 2 e^{-\gamma_E}$ and $\nu=\omega$. Note that with this choice of scales, the displayed beam function is the boundary term of a resummed prediction.}
 \label{fig:ratio_to_LO}
\end{figure*}

In order to understand the impact of the new three-loop boundary term $\tilde I_{ij}^{(3)}$ in a resummed predictions, we present the beam function evaluated at the canonical scales $\mu b_T = 2 e^{-\gamma_E}$ and $\nu = \omega$, where all logarithms in \eq{logdef} vanish and only the boundary term $\tilde I_{ij}^{(3)}$ contributes.
In \fig{ratio_to_LO}, we compare the $u$-quark beam function (left) and gluon beam function (right) order by order in $\alpha_s$, up to N$^3$LO, to the corresponding PDFs, choosing canonical scales for $b_T = (10~\,\mathrm{GeV})^{-1}$ and $\omega=100~\,\mathrm{GeV}$.
We see that the beam function has a very different shape compared to the PDF, and that the beam function converges very well at N$^3$LO.

\begin{figure*}
 \centering
 \includegraphics[width=0.55\textwidth]{plots/Kfactor_udg.pdf}
 \caption{The $K$-factor of the N$^3$LO beam function, i.e.\ the ratio of the N$^3$LO beam function to NNLO beam function. We fix $b_T = (10~\,\mathrm{GeV})^{-1}$ and $\omega=100~\,\mathrm{GeV}$ and choose the canonical scales $\mu b_T = 2 e^{-\gamma_E}$ and $\nu=\omega$, such that the shown beam function corresponds to the boundary term in a resummed prediction. The different colors show the results for an $u$-quark, $d$-quark and gluon, respectively.}
 \label{fig:Kfactor}
\end{figure*}

Finally, the $K$-factor of the N$^3$LO beam function, which is defined as the ratio of the beam function at N$^3$LO w.r.t. its value at NNLO, is shown in \fig{Kfactor}.
As before, we choose the canonical scales for $b_T = (10~\,\mathrm{GeV})^{-1}$ and $\omega=100~\,\mathrm{GeV}$.
We find a rather small correction of $\sim 0.2-0.5\%$, but with a notable dependence on $z$ for all channels.

For completeness, we also present the high-energy limit $z\to0$ of the kernels $\tilde I_{gg}^{(3)}(z)$ and $\tilde I_{gq}^{(3)}(z)$ contributing to the gluon beam function in \app{high_energy}. The corresponding limit for the quark kernels were already presented in \refcite{Luo:2019szz}, for which we find perfect agreement.
These results are useful to study the small-$x$ behavior of TMDPDFs, see e.g.~\refscite{Balitsky:2015qba,Marzani:2015oyb,Balitsky:2016dgz,Xiao:2017yya}.

\section{Conclusions}
\label{sec:conclusion}

We have calculated the perturbative matching kernel relating transverse-momentum dependent beam functions with lightcone PDFs at N$^3$LO in QCD.
This provides the first results of these kernels for the gluon TMD beam function, and corrects the result in the $d_{abc} d^{abc}$ color structure in the recent calculation of the quark TMD beam function in \refcite{Luo:2019szz}.
After private communication, the authors of~\refcite{Luo:2019szz} identified and resolved a minor mistake in their calculation, after which perfect agreement is found.
This emphasizes that having two independent computations that are in accordance with each other is the most stringent cross check.
Our results are obtained via a framework recently developed by us that allows for the efficient expansion of differential hadronic collinear cross sections~\cite{Ebert:2020lxs}, showing its applicability for the extraction of universal ingredients arising in the collinear limit of QCD to an unprecedented level of precision in perturbation theory.
As a byproduct, we also confirmed a previous computation of the soft function for transverse momentum factorization~\cite{Li:2016axz}.

The results of our calculation are provided in the ancillary files of this paper submission. We include, for all quark and gluon channels, the renormalized TMD beam functions, along with their expansions around $z=0$ and $z=1$ up to 50 orders in each expansion, as well as the renormalized TMDPDFs and the bare and renormalized soft function.

The phenomenological applications of our results are numerous.
Firstly, we provide the last missing ingredient for the fully-differential calculation of color-singlet processes at N$^3$LO using the $q_T$ subtraction method~\cite{Catani:2007vq,Cieri:2018oms,Billis:2019vxg}, which can be used to obtain the first exact fully-differential cross sections at this order.
They also enable the resummation of transverse momentum distributions at hadron colliders at N$^3$LL$^\prime$ accuracy, both for gluon and quark induced hard scatterings such as Higgs-boson production and the Drell-Yan process, two key observables at the LHC.

A natural future direction of this research is the calculation of the closely related TMD fragmentation functions at N$^3$LO, which are required to describe the small-$q_T$ limit semi-inclusive deep inelastic scattering and are currently only known at NNLO \cite{Echevarria:2016scs,Luo:2019bmw,Luo:2019hmp}.

With the same techniques presented in this work, it would also be interesting to consider the calculation of other ${\vec q}_T$-dependent time-like collinear functions, such as the Energy-Energy Correlator (EEC) jet functions.
The quark and gluon EEC jet functions enter the factorization of the EEC in the back-to-back limit for $e^+e^-$ annihilation and gluon initiated Higgs decay, respectively~\cite{Moult:2018jzp}, as well as that for the TEEC~\cite{Gao:2019ojf}.
Their knowledge at N$^3$LO is the only missing ingredient to achieve resummation of the EEC in the back-to-back limit at N$^3$LL$^\prime$ accuracy. Note that at fixed order the full angle EEC has been calculated analytically through $\mathcal{O}(\alpha_s^2)$ \cite{Dixon:2018qgp,Luo:2019nig}.

It will also be interesting to study the collinear expansions beyond leading power to shed light on the structure of TMD factorization at subleading power, in particular on the structure of rapidity divergences at subleading power~\cite{Moult:2017xpp,Ebert:2018gsn,Moult:2019vou}.

\acknowledgments
We thank the Ming-xing Luo, Tong-Zhi Yang, Hua Xing Zhu and Yu Jiao Zhu for private communication concerning the results of \refcite{Luo:2019szz} prior to the publication of this article that allowed both groups to agree on our results.
We also thank Johannes Michel, Iain Stewart and Frank Tackmann for useful discussions.
This work was supported by the Office of Nuclear Physics of the U.S.\ Department of Energy under Contract No.\ DE-SC0011090 and DE-AC02-76SF00515, and within the framework of the TMD Topical Collaboration.
M.E.\ is also supported by the Alexander von Humboldt Foundation through a Feodor Lynen Research Fellowship,
and B.M.\ is also supported by a Pappalardo fellowship.

redpajama_set_name: RedPajamaArXiv


text:
Oldham sign Wigan academy winger
By Jack Conlon October 16, 2020 mode_comment0
Oldham have confirmed the signing of Wigan academy winger Ben Holcroft on a one-year deal from 2021.
The 19-year-old has progressed through the Warriors' scholarship, academy and reserves systems, with a highlight being scoring a try in his side's Super League Academy Grand Final win over St Helens last year (above).
He becomes the Roughyeds' seventh new signing for next season, following the acquisitions of Shaun Pick, Luke Nelmes, Tyler Dupree, Tommy Brierley, Ben Heaton and Martyn Reilly.
"It will be a big leap out of my Wigan comfort zone, but I know John Hutchings and some of the other lads who are already at Oldham and that will help me to settle in," Holcroft said. "I'm really looking forward to being part of the Oldham squad and getting the chance to show what I can do."
"I loved my years at Wigan, but it was time to move on and seek a new challenge and Oldham convinced me it was the club for me.
"I played centre when I first went to Wigan on scholarship, but my coach at that time said he preferred me on the wing and I've been on the wing ever since."
Oldham head coach Matt Diskin added: "He's a big lad for an outside back and he'll be pushing for a wing spot. Occupancy of the wing positions is still up in the air at the moment and Ben will have just as much chance as anybody else.
"He's very strong with the ball coming out of backfield and that's essential for a winger in the modern game.
"If he works hard, adapts to the change and strives hard to reach personal goals as well as those of the team and the club he'll do well, of that I have no doubt."


P5 Viking Showcase was outstanding – a great celebration of all the expressive arts the children do in class. Great parental engagement too, it is definitely one of the best ways to find out and share learning with lots of children in the class. Well done everyone in P5!
Sharing the learning: This week P2s have been sharing all they have been learning about stars with me. I was very impressed in the knowledge they learned, but even more by the way they were able to explain how they were learning and what they wanted to learn next. Full marks for engagement and enthusiasm P2!
On Friday night 60 boys and girls, with 11 Bruntsfield parents, raised £3,700 for Social Bite at the 'Wee Sleep'. They slept in survival bags, without tents, at Bonaly outdoor centre. I am told, the weather wasn't too kind, it rained almost all night! Thanks to the Cubs and Scouts from 100th Pentland who led this great adventure.
It was a pleasure to present the first Bronze JASS (Junior Awards Scheme for Schools) Certificates and Badges of the session. Awards were given for good Citizenship, outdoor learning and contribution to our community, this programme is part of our P6/ P7 curriculum.
New South Edinburgh Primary School (Canaan Lane) Update: The Council are proposing that the new primary school will open from August 2021, with registration in November 2020 to allow P1 classes and any upper stage classes to start in the new building at the same time in August 2021. There will be no mandatory transfer of pupils already attending another school. Current catchment arrangements will continue to apply for registrations in November 2019. An email with further details has been sent to you.
P1 and P2 outdoor learning: teachers may take their children to our local environment at any time and excursions to woodlands are booked for next term, which the teachers will build on, details to come from class teachers nearer the time. Parent helpers are always in demand, please liaise with your class teachers if you would like to be involved.
Parent Class Reps: I shall remind the staff how helpful you are for sharing information, especially in the run up to trips and events. If you are a class rep, please make contact with your class teacher.
Relationship with Barclay Viewforth Church: Each school in the city is matched with a Church within their community. Bruntsfield historically worked with both Barclay and Viewforth Churches. When they merged, we remained associated with what is now called Barclay Viewforth Church. Rev Sam Torrence visits us once a month and shares our Assemblies based on the Rights of the Month. As school numbers have grown, it has not been possible to have all the children visit Church together, once a year at the same time the way we used to. Hence the reason P1 lead Christmas Celebrations, P3 Harvest and P5 Easter. P7s join and help the P1s, P2 and P4 join Harvest and P6 join the Easter Celebration.
Quiet spaces at break and lunch: the team working on the playground identified the picnic areas as the best place for quieter games and story telling. Reminding everyone of this shall be a priority.
ParentPay: please review your notifications and preferences, the default is set to 'no alerts'. Please be aware, this may mean you may miss messages and invoices, unless you go into your account.
1+2 Language Programme: this was discussed at the Cluster Head Teacher meeting this week and our Cluster Primary Schools shall continue with French from P1-P7 in addition to Mandarin in P5 and German in P6 and P7. P1-P4 children learn one language and P5-P7 children learn 2 languages. It generally works out at one hour per week. Best practice is when languages are used during the day as part of their ongoing learning and consolidation. 'Phrases of the week' build confidence and discussions across the school. Boroughmuir currently continue both French and German in SI. They do offer an option of Mandarin if you prefer. This year's S1 have two periods of French and one of German for part of the year, then swap, having two periods of German and one of French, this balances across the year. This is reviewed annually by the Cluster Head Teachers and we add any changes to the Improvement Plan. Staff who lead languages across the four schools have all worked together and followed an agreed programme for each language, in line with the City plan for languages.
Assessments (testing): Assessments are used to confirm teacher judgements on progress and help teachers plan next steps in learning, ensuring all children are challenged and supported. P4 and P7 assessments from the Scottish Government are completed by the pupils on line and schools are not given copies in advance or afterwards, therefore we are unable to share them with you.
Home Learning Policy: We have updated the website to show this is now finalised and no longer in draft form. Thank you to all who helped contribute to this.
P7 Memory Boxes: I have shared the feedback from you with the teachers, thank you.


text:
Smasher:ononox
ononox "おののっくす"
Palutena, Greninja
ononox (おののっくす) is a Super Smash Bros. for Wii U Cloud player from Japan. ononox has taken sets off of players such as Takashi and Nojinko.
ononox also mains Cloud in Ultimate and has defeated players like Yazawa, Lucia, Injelly, Nanchan, TOSHI, and Alex.
Karisuma 2 February 14th, 2015 49th — —
Karisuma 3 May 23rd, 2015 33rd — —
Karisuma 4 July 25th, 2015 25th — —
Karisuma 5 October 10th, 2015 65th — —
Karisuma 6 April 3rd, 2016 49th — —
Karisuma 8 June 25th, 2016 49th — —
Sumabato for THE BIG HOUSE July 30th-31st, 2016 97th — —
Sumabato 13 September 25th, 2016 65th — —
Karisuma 10 October 8th, 2016 33rd — —
Karisuma 11 November 26th, 2016 33rd — —
Karisuma 13 April 23rd, 2017 49th — —
Karisuma 14 June 24th, 2017 33rd — —
Umebura T.A.T. December 23rd, 2017 113th — —
Umebura 32 May 12th, 2018 129th — —
Sumabato 26 June 30th, 2018 49th — —
Umebura 34 August 25th, 2018 193rd — —
Sumabato SP January 6th, 2019 65th — —
Karisuma SP 1 January 12th, 2019 33rd — —
Sumabato SP 2 February 2nd, 2019 49th — —
Sumabato SP 3 April 14th, 2019 65th — —
Umebura Japan Major 2019 May 1st-2nd, 2019 257th — —
Karisuma SP 2 May 18th, 2019 25th — —
Sumabato SP 4 May 26th, 2019 97th — —
Gifu smash 7 June 27th, 2019 7th — —
Sumabato SP 7 August 12th, 2019 65th — —
Sumabato SP 8 September 15th, 2019 65th — —
Sumabato SP 10 December 15th, 2019 65th — —
Maesuma TOP 1 January 4th, 2020 65th — —
Toyota Taisenkai 8 February 1st, 2020 17th — —
Maesuma TOP 2 March 1st, 2020 97th — —
Maesuma TOP 4 October 31st-November 1st, 2020 49th 9th DIO
Karisuma SP 10 November 14th, 2020 9th — —
Mēsuma November 29th, 2020 25th — —
Toyota Grand Slam 3 March 14th, 2021 9th — —
Gifu smash 13 April 12th, 2021 5th — —
Toyota Grand Slam 4 April 17th, 2021 13th — —
Maesuma TOP 5 July 3rd-4th, 2021 49th 5th DIO
Miesuma SP 6 July 24th, 2021 7th — —
Gifu smash 14 August 7th, 2021 9th — —
FCTZS Cup August 8th, 2021 17th — —
Maesuma TOP 6 October 22nd, 2021 65th — —
Umabura SP 1 November 6th, 2021 13th — —
Miesuma SP 7 December 4th, 2021 9th — —
Mēsuma 2 December 12th, 2021 33rd — —
Miesuma SP 8 December 19th, 2021 9th — —
Kagaribi 6 Jamuary 8th-9th, 2022 129th — —
Gifu Smash x C-Sea January 16th, 2022 17th — —
Retrieved from "https://www.ssbwiki.com/index.php?title=Smasher:Ononox&oldid=1652708"
Chūbu smashers
Cloud professionals (SSBU)
This page was last edited on January 16, 2022, at 13:27.


" Dear Students, the fact that you are browsing the pages of this document is reflective of your interest in becoming part of this institution. I wish that you make an intelligent and correct decision in selecting a field of studies leading to the profession as your future career.While making this decision I am sure that you would have had complete information about Qurtuba University generally and the Faculty of Engineering particularly.
Under the Faculty of Engineering, three degree programs namely Electrical Engineering, Civil Engineering and B-Tech Engineering are being offered at the Dera Ismail Khan campus of the University.
All the disciplines are having well equipped laboratories and highly qualified, experienced and dedicated faculty. This fact is recognized by the Pakistan Engineering Council, the statutory body that accords the accreditation and recognition to the engineering qualification and profession.
Civil Engineering and mankind advancement go side by side since medieval ages. In computer age and technological advancements in the design, construction, and maintenance of civil infrastructure have made this field even more important. The BSc Civil Engineering degree program at the Qurtaba University of Science and Technology D.I.Khan Campus is designed to prepare competent professional Civil Engineers with special emphasis on basic civil engineering theory coupled with practical training to meet the challenges of market. Particular attention is paid to tune the important subjects such as Structural Engineering, Transportation Engineering, Geo technical Engineering, Environmental Engineering, Surveying and Water Resources Engineering.
Recognize and define Civil Engineering problems and suggest practical solutions using up to date Civil Engineering practices.
Practical application of knowledge of science and Civil Engineering in their professional career.
Design Civil Engineering projects using the standard procedures for accomplishing such work.
Design, conduct and interpret the results of Civil Engineering field and experimental data.
Work effectively in diverse teams and provide leadership to teams and organization.
Express effectively using verbal, graphic and written forms of communication.
Understand the impact of engineering decisions in social, economic, environmental and global context.
Adhere to discipline and code of ethics of engineering profession.
Engage in life-long learning and recognize the importance of doing so.
A broad education necessary to contribute effectively beyond their professional careers.
Civil Engineers/Technlogists are employed in diversified sectors of the society ranging from government departments to architectural and town planning firms, builders, and engineering firms in the private sector. There are also career options available in education and research and development (R&D). Civil Engineers/Technlogists often work at construction sites and infrequently in offices and testing labs. Graduates will have ample opportunities of getting jobs in various departments e.g. Communication & Works (C&W), Water and Power Development Authority (WAPDA), FATA Development Authority, Civil Aviation Authority (CAA), Pakistan Railways (PR), National Highway Authority (NHA), Peshawar Development Authority (PDA), KPK Public Health Engineering Department, National Engineering Services Pakistan (NESPAK), and many more private consultants.
Student of Civil Engineering/Technology will be required to carry out a mandatory field training in surveying through a Survey Camp, arranged for three weeks duration. The field training will cover comprehensively the contouring, triangulation, leveling and plan table survey under the supervision of survey experts. Completion of this training is mandatory for the award of BSc Engineering/B-Tech degree. After successful completion of training, the student will be awarded a Survey Training Course certificate.


text:
Q: Not able to send packets in scapy on python3/Mac OS I am new to scapy and was trying to send an icmp packet using my wireless interface. I keep getting following error. I am using the latest scapy version on python3.  When i try to send packet using python3 shell i keep getting segmentation fault 11 error. Both sr and send is failing.
bash-3.2$ ifconfig en1
en1: flags=8863<UP,BROADCAST,SMART,RUNNING,SIMPLEX,MULTICAST> mtu 1500
ether 24:a0:74:ef:c2:0a
inet6 fe80::1421:2877:9b9f:8b7e%en1 prefixlen 64 secured scopeid 0x5
inet 192.168.0.56 netmask 0xffffff00 broadcast 192.168.0.255
nd6 options=201<PERFORMNUD,DAD>
media: autoselect
status: active
bash-3.2$ ping -S 192.168.0.56 www.google.com
PING www.google.com (172.217.166.68) from 192.168.0.56: 56 data bytes
64 bytes from 172.217.166.68: icmp_seq=0 ttl=55 time=26.458 ms
64 bytes from 172.217.166.68: icmp_seq=1 ttl=55 time=21.927 ms

bASH-3.2$ scapy
WARNING: Cannot read wireshark manuf database
WARNING: Crypto-related methods disabled for IPsec, Dot11 and TLS
         layers (needs python-cryptography v1.7+).
WARNING: No route found for IPv6 destination :: (no default route?)
INFO: Can't import python-cryptography v1.7+. Disabled WEP
decryption/encryption.
INFO: Can't import python-cryptography v1.7+. Disabled IPsec
encryption/authentication.
WARNING: IPython not available. Using standard Python shell instead.
AutoCompletion, History are disabled.

                   aSPY//YASa
           apyyyyCY//////////YCa       |
          sY//////YSpcs  scpCY//Pp     | Welcome to Scapy
 ayp ayyyyyyySCP//Pp           syY//C    | Version 2.4.0rc4
 AYAsAYYYYYYYY///Ps              cY//S   |
     pCCCCY//p          cSSps y//Y   | https://github.com/secdev/scapy
     SPPPP///a          pP///AC//Y   |
          A//A            cyP////C   | Have fun!
          p///Ac            sC///a   |
          P////YCpc           A//A   | To craft a packet, you have to be a
   scccccp///pSP///p          p//Y   | packet, and learn how to swim in
  sY/////////y  caa           S//P   | the wires and in the waves.
   cayCyayP//Ya              pY/Ya   |        -- Jean-Claude Van Damme
    sY/PsY////YCc          aC//Yp    |
     sc  sccaCY//PCypaapyCP//YSs
              spCPY//////YPSps
                   ccaacs

>>> sr(IP(dst='www.google.com')/ICMP())
Traceback (most recent call last):
File "<console>", line 1, in <module>
File "/Library/Python/2.7/site-packages/scapy-2.4.0rc4-
py2.7.egg/scapy/sendrecv.py", line 364, in sr
s = conf.L3socket(promisc=promisc, filter=filter, iface=iface,
nofilter=nofilter)
File "/Library/Python/2.7/site-packages/scapy-2.4.0rc4-
py2.7.egg/scapy/arch/bpf/supersocket.py", line 57, in __init__
(self.ins, self.dev_bpf) = get_dev_bpf()
File "/Library/Python/2.7/site-packages/scapy-2.4.0rc4-
py2.7.egg/scapy/arch/bpf/core.py", line 98, in get_dev_bpf
raise Scapy_Exception("No /dev/bpf handle is available !")
Scapy_Exception: No /dev/bpf handle is available

A: Try it with sudo scapy, it worked for me.
Here where I found the solution:
https://github.com/secdev/scapy/issues/1343
guedou commented on 8 Sep  Scapy needs to be run as root to send
packets.

A: I ran into this same issue, but also for just sniffing packets (i.e., not to send, which I know needs root). So just starting scapy and running >>> sniff() would return Scapy_Exception: No /dev/bpf handle is available.
It turns out that by default the /dev/bpf* devices are owned by wheel, which my regular user is not part of. This is why sudo scapy works. The issue is that running under sudo is not always convenient.
I don't know if the /dev/bpf* devices be owned by any other group, but a quick workaround indicates that they can ...
Just install Wireshark! Once wireshark is installed, the /dev/bpf* devices are owned by access_bpf, a group that the non-root user is added into.

A: I got the same issue running with scapy as user with admin rights on Mac.
The solution is to run as super user - sudo
I tried it on both python 2.7.17 and 3.7.6.
Make sure you have the updated scapy package, see installation instruction on https://scapy.readthedocs.io/en/latest/installation.html
The root admin rights for scapy are listed in the following github issue doc https://github.com/secdev/scapy/issues/1851

redpajama_set_name: RedPajamaStackExchange


text:
Sensor technology, Communications technology
Artificial satellite
SATCOM 47, a late 20th century communications satellite orbiting Earth
A display of a network of artificial satellites
For natural satellite, please see moon.
An artificial satellite was a man-made form of technology that was put in orbit around a planet. (VOY: "Future's End, Part II") They had countless applications, including defense, weather forecast, surveillance, and communication, and were used by many cultures.
Earth Edit
Earth launched its first artificial satellite, Sputnik, in 1957. This milestone was monitored by a Vulcan team. (ENT: "Carbon Creek")
T'Mir's statement that "It's hard to believe these people were capable of launching an artificial satellite" might suggest that species generally launched their first satellite later in their history.
By 1968, weather satellites were used. (TOS: "Assignment: Earth")
By the late 20th century, the cryonics fad had resulted in cryonics satellites being put into Earth's orbit. (TNG: "The Neutral Zone")
According to Tom Paris, by 1996 Earth had surveillance satellites in orbit. Satellite dishes were in use for communication with satellites. (VOY: "Future's End")
In 2024, news services used satellite images to assess what was happening in Sanctuary District A during the Bell Riots. The images showed a number of potential casualties. (DS9: "Past Tense, Part II")
By 2154, Starfleet Operations operated a grid of satellites in Earth orbit, capable of picking up any transporter activity on the planet. (ENT: "Affliction")
Vulcan Edit
In 2097, the Vulcan High Command put a surveillance satellite in orbit of Weytahn to monitor potential violations of the Treaty of 2097. (ENT: "Cease Fire")
By 2154, Vulcan had a network of security satellites in orbit, providing satellite surveillance. (ENT: "Awakening")
United Federation of Planets Edit
By the second half of the 24th century, Earth relied on a network of satellites for communications. (DS9: "Past Tense, Part I") Navigational control satellites were also in use, one of which was in orbit of Saturn. (TNG: "The First Duty")
By 2370, the Prytt Alliance became concerned that the Federation was helping the Kes to develop attack satellites, and claimed to have developed countermeasures. (TNG: "Attached")
By 2372, the Federation had deployed a relay satellite on the Gamma Quadrant side of the Bajoran wormhole. (DS9: "Paradise Lost")
Other species Edit
Lazarus claimed to have survived the destruction of his civilization by being occupied with inspecting magnetic communications satellites when the destruction occurred. (TOS: "The Alternative Factor")
A Xindi-Arboreal colony visited by Enterprise in 2153 had no artificial satellites. (ENT: "The Shipment")
Satellites were used to generate the dispersion field protecting parts of the Torothan homeworld from orbital scans. (ENT: "Desert Crossing")
by 2151 Valakis had many satellites in orbit. (ENT: "Dear Doctor")
In 2153, the Azati Prime system featured a extremely sensitive security net, provided by a large array incorporating thousand of satellites. (ENT: "Azati Prime")
By 2267, the Eminian Union was using tricobalt satellites in the Eminiar-Vendikar War. (TOS: "A Taste of Armageddon")
Sometime before the destruction of the Vaadwaur homeworld in 1484, the Vaadwaur put a sentry satellite in geostationary orbit above one of their cities. (VOY: "Dragon's Teeth")
A Kohl settlement devastated by solar flares in 2353 was still orbited in 2372 by several by then-nonfunctional communications satellites. (VOY: "The Thaw")
In 2366, the Romulans claimed to be doing archaeological research on Nelvana III, using a cloaked satellite. (TNG: "The Defector")
A moon located in the Gamma Quadrant was orbited by a network of artificial satellites which attacked starships nearby and protected the imprisoned Ennis and Nol-Ennis. (DS9: "Battle Lines")
By 2373, Taresia was defended by a high-density polaron grid generated by a network of satellites. (VOY: "Favorite Son")
By 2376, the orbit of the Qomar homeworld was so filled with spaceships and satellites that entering it felt like navigating an obstacle course. (VOY: "Virtuoso")
List of artificial satellites Edit
SATCOM 47 (orbited Earth, late 1990s)
Sputnik I (orbited Earth, mid 1950s)
Surveillance and research
Spy satellite
Security satellite (also known as recon satellite, sentry satellite, or surveillance satellite)
Monitor beacon satellite (2120s)
Communication and navigation
Navigational control satellite (2360s)
Federation communications satellite (2360s)
Relay satellite (2372)
Magnetic communication satellite
Tricobalt satellite
Attack satellite (2370 - possibly only theoretical)
Cryonics satellite
Ultraviolet satellite (2260s)
Co-orbital satellite
Appendices Edit
Satellite surveillance
Satellite grid
Midos V Satellite City Spaceport
Satellites seem so common in the Star Trek universe that their absence was an indicator that the planet did not harbor a warp-capable civilization (for example, in "Strange New World", "Civilization", or "Time and Again"), or alternatively that a planet was only a minor outpost (for example in "The Shipment").
Satellite at Wikipedia
Retrieved from "https://memory-alpha.fandom.com/wiki/Artificial_satellite?oldid=1942113"
Communications technology
1 Phaser
2 Repression (episode)
3 Star Trek: The Official Starships Collection


text:
SPONSOR Hawley (MS)
COSPNSR Crouch, Giglio, Palmesano, Salka, Lawrence
MLTSPNSR Thiele
Amd Part LL-1 §1, Chap 57 of 2008; amd §1134, Tax L
Prohibits the New York state department of taxation and finance from charging a fee for applications for a certificate of registration pursuant to a re-registration program.
01/17/2019 referred to ways and means
A01762 Committee Votes:
A01762 Floor Votes:
There are no votes for this bill in this legislative session.
Introduced  by M. of A. HAWLEY, CROUCH, GIGLIO, PALMESANO -- Multi-Spon-
sored by -- M.  of A. THIELE -- read once and referred to the  Commit-
tee on Ways and Means
AN  ACT  to  amend  section  1 of part LL-1 of chapter 57 of the laws of
2008, relating to directing the commissioner of taxation  and  finance
to institute a re-registration program, in relation to prohibiting the
New  York  state  department  of  taxation and finance from charging a
vendor re-registration fee; to authorize the refund of  all  re-regis-
tration  fees  collected  by the New York state department of taxation
and finance; and to amend the tax law, in relation to prohibiting  the
New  York  state  department  of  taxation  and  finance from charging
vendors any fees to collect NYS sales tax
1    Section  1.  Section 1 of part LL-1 of chapter 57 of the laws of 2008,
2  relating to directing the commissioner of taxation and finance to insti-
3  tute a re-registration program, is amended to read as follows:
4    Section 1.  The commissioner of taxation and finance  is  directed  to
5  institute  a re-registration program pursuant to section 1134 of the tax
6  law, which program should be completed by March  31,  2012.    [Notwith-
7  standing  any  law  to  the  contrary, every certificate of registration
8  filed pursuant to this re-registration program by a person  required  to
9  file sales and compensating use tax returns for the monthly or quarterly
10  periods  described in section 1136 of the tax law must be accompanied by
11  a 50 dollar application fee to constitute a complete  application.  This
12  fee must be paid and disposed of in the same manner as the taxes imposed
13  by  section  1105  of  the  tax  law  and  may  be determined, assessed,
14  collected and enforced in the same manner as the tax imposed by  article
15  28  of  the tax law. Notwithstanding section 1148 of the tax law, or any
16  other law to the contrary, such commissioner must retain from the appli-
17  cation fees collected or  received  an  amount  that  such  commissioner
1  determines  is  necessary to cover reasonable costs of such commissioner
2  in implementing, administering and enforcing registrations  pursuant  to
3  this  section, but no more than the amount of those fees. The provisions
4  of subdivisions (a) and (c) of section 1139 of the tax law apply, except
5  that  no  interest  is  allowed  or paid on any refund.] A person may be
6  subject to the re-registration program directed by this section even  if
7  such person holds a certificate of authority that has not been in effect
8  for a period of at least three years.
9    §  2. Notwithstanding any law, rule or regulation to the contrary, all
10  50 dollar application fees collected by the department of  taxation  and
11  finance  pursuant  to  the  re-registration  program  instituted  by the
12  commissioner of taxation and finance as authorized by section 1 of  part
13  LL-1  of chapter 57 of the laws of 2008 shall be refunded to the persons
14  who paid such fees.
15    § 3. Paragraph 5 of subdivision (a) of section 1134 of the tax law, as
16  amended by chapter 2 of the laws of 1995, is amended to read as follows:
17    (5) If the commissioner considers it necessary for the proper adminis-
18  tration of the sales and use taxes and prepaid  taxes  imposed  by  this
19  article  and  pursuant  to  the authority of article twenty-nine of this
20  chapter, it may require every  person  under  this  section  or  section
21  twelve  hundred  fifty-three  of this chapter who holds a certificate of
22  authority to file a new certificate of registration, without charge, and
23  in such form and at such time as the commissioner may prescribe  and  to
24  surrender  such  certificate  of authority. The commissioner may require
25  such filing and such surrender not more  often  than  once  every  three
26  years.  Upon  the  filing  of  such  certificate of registration and the
27  surrender of such  certificate  of  authority,  the  commissioner  shall
28  issue, within such time as the commissioner may prescribe, a new certif-
29  icate  of  authority, without charge, to each registrant and a duplicate
30  thereof for each additional place of business of such registrant.
31    § 4. This  act  shall  take  effect  immediately;  provided  that  the
32  provisions of section two of this act shall apply to all certificates of
33  registration  required  to  be  filed  under section 1134 of the tax law
34  pursuant to the re-registration program instituted by  the  commissioner
35  of taxation and finance as authorized by section 1 of part LL-1 of chap-
36  ter 57 of the laws of 2008 and filed on or after November 1, 2008.


text:
using System;
using System.IO;
using System.Collections.Generic;
using System.Linq;
using System.Text;

namespace netlint.framework
{
	class Accumulator
	{
		List<string> missing = new List<string>();
		List<string> extra = new List<string>();
		private IList<string> files;
		private string baseDir;
		private IFileGlobber globber;
		private string projectFile;
		private Logger logger;

		public Accumulator(string baseDir, IList<string> files, IFileGlobber globber, string projectFile, Logger logger)
		{
			this.baseDir = baseDir;
			this.files = files.Select(x => new FileInfo(Path.Combine(baseDir, x)))
				.Select(x => x.FullName).ToList();
			this.globber = globber;
			this.projectFile = projectFile;
			this.logger = logger;
		}

		public void Execute()
		{
			foreach (var name in files)
			{
				var file = Path.Combine(baseDir, name);
				if (!File.Exists(file))
				{
					missing.Add(file);
				}
			}

			Walk(new DirectoryInfo(baseDir));

			if (missing.Any() || extra.Any())
			{
				var ex = new NetLintProjectScanException(projectFile, missing, extra);
				logger.Log(ex.Message);
				throw ex;
			}
		}

		private void Walk(DirectoryInfo current)
		{
			var lowered = files.Select(x => x.ToLowerInvariant());
			foreach (var f in Directory.GetFiles(current.FullName)
				.Where(x => globber.ShouldCheckFile(x) && !lowered.Contains(x.ToLowerInvariant())))
			{
				extra.Add(f);
			}

			foreach (var dir in current.GetDirectories())
			{
				if (!globber.IsDirIgnored(dir.FullName))
				{
					Walk((DirectoryInfo)dir);
				}
			}
		}
	}
}

redpajama_set_name: RedPajamaGithub


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Poonam Bajaj and Shuxiang Liu are recipients of Outstanding Student Award.
Ravi Kiran Tadapaneni, Ellen Bornhorst, Jungang Wang and Deepali Jain are recipients of Travel award.
Hongchao Zhang is recipient of Scholastic Award.
The awards were presented to recipients at the Student Awards Dinner on Thursday May 12th in Seattle by PSIFT.


This free app enables you to gain unlimited access to live broadcasts and radio stations from Philippines. Feel free to enjoy music, news and live radio broadcasting anytime and anywhere with the well-connected network. No matter you are on a bus or a train, the network is hardly interrupted. No worries.
Note: Not all the live streams are embedded with metadata.


This is a staple recipe that is easy, delicious and nutritious! The main ingredients are crushed tomatoes and garbanzo beans.
Bring a big pot of water to a boil for the pasta. Cook to al dente. While the spaghetti cooks, heat a large skillet over medium heat. Place the chickpeas and garlic in a processor and pulse to a fine chop. Heat oil in a skillet- add the chickpeas to the skillet with the and season with salt and pepper. Saute for 3-4 minutes. Add the wine or broth and cook down for 30 seconds or so, then stir in the tomatoes. Drain the pasta and toss with the sauce. Top the pasta with parsley and grated cheese.
Nutrition Note: Beans count as a vegetable as well as a source of protein. Beans are an excellent source of fiber, protein, potassium, folate, and magnesium. They have been linked to lowering LDL (the bad) cholesterol, high blood pressure and reduced risk of heart disease, improving blood sugar regulation and reducing risk of certain cancers. If you have difficulty digesting beans try incorporating them gradually ie 1/4 c – 1/2 cup serving size.


In the Kurdish capital, Arbil, traffic wardens issue parking tickets, foreign businessmen relax in newly built hotels and gunfire is seldom heard.
But while security conditions are favourable here, Kurds are reluctant to press ahead with polling while the rest of Iraq is in turmoil. There is unease that the US-appointed government is rushing towards elections.
"If everybody wanted elections to go ahead in our area there would be no problems and everything would happen normally," said Ahmed Abdulwahid, a senior member of the Kurdish parliament in Arbil.
Kurdish factions have been running their own affairs ever since the first Gulf war in 1991 forced Iraqi forces to pull out of the area, holding their own elections in 1992 and building up an army of around 70,000 soldiers known as "peshmerga".
The peshmerga (meaning "those ready to die") fought alongside US forces during the 2003 invasion. Afterwards they were transformed into the local security forces and have prevented violence spilling into the Kurdish territory.
But Kurds face an uncertain future. Many in Arbil fear an Arab-dominated government in Baghdad will curtail the freedoms they achieved after decades of oppression.
Under Saddam's regime, more than 100,000 Kurds were killed or taken away by Iraqi security forces and never seen again. The memory of Iraqi planes dropping gas bombs on Kurdish villages makes Kurds distrustful of ceding authority to Baghdad.
"We want a central government and stability for all Iraq, but Kurds must have a significant role so that we are protected," said 29-year-old Farouq Abdulgheni, seated behind the counter of a busy grocery store.
In a deal struck in Baghdad on March 18, 2003, Kurds ensured their right to federal autonomy was enshrined in the new constitution of Iraq. Kurdish leaders insisted on retaining a degree of control over their own territory.
Even this resolution was regarded as a compromise and many Kurds see federalism as simply a step towards their dream of creating an independent state, but central to this plan is the inclusion of the oil-rich city of Kirkuk within the Kurdish zone.
Kurds claim the city's population was predominantly Kurdish before Saddam's "Arabisation" campaign – deporting the Kurds and replacing them with Arabs from the country's south – to change the city's demographic structure, thus safeguarding his control of Iraq's largest oilfields.
But following the US-led invasion, more than 100,000 Kurds returned to Kirkuk and are now living in refugee camps in and around the city, creating friction with Kirkuk's large Arab and Turkomen communities.
Kurdish politicians are determined that Arabisation should be reversed and Kurdish refugees allowed to vote in the upcoming elections to determine the city's status, yet the issue remains unresolved.
"Pre-existing questions such as the 'normalisation' of Kirkuk have not been addressed, so it is not logical for this election to go ahead at the appointed time," said parliamentarian Abdulwahid. Control of Kirkuk is vital to Kurdish hopes of self-determination and Kurdish leaders have frequently stated they won't compromise on this.
In the marketplaces and cafés of downtown Arbil, conversations are dominated by the issue. "Kurds were kicked out of Kirkuk and the Arabs were brought in by Saddam," said Kurdish labourer Shawkat Denha, 42, sipping a glass of black tea.
Watching the violence in the rest of Iraq, many Kurds are sceptical about the chances of holding elections outside the Kurdish zone – most acknowledge that a delay could work in their favour.
"Holding elections on time would be a blow to those trying to destabilise Iraq," said Abdulwahid.