Article
Reference
Two-particle momentum correlations in jets produced in pp collisions at s√=1.96 TeV
CDF Collaboration
CLARK, Allan Geoffrey (Collab.), et al.
Abstract
We present the first measurement of two-particle momentum correlations in jets produced in pp collisions at s√=1.96 TeV. Results are obtained for charged particles within a restricted cone with an opening angle of 0.5 radians around the jet axis and for events with dijet masses between 66 and 563 GeV/c2. A comparison of the experimental data to theoretical predictions obtained for partons within the framework of resummed perturbative QCD in the next-to-leading log approximation shows that the parton momentum correlations survive the hadronization stage of jet fragmentation, giving further support to the hypothesis of local parton-hadron duality. The extracted value of the next-to-leading-log-approximation parton shower cutoff scale Qeff set equal to ΛQCD is found to be (1.4+0.9−0.7)×100 MeV.
CDF Collaboration, CLARK, Allan Geoffrey (Collab.), et al . Two-particle momentum correlations in jets produced in pp collisions at s√=1.96 TeV. Physical Review. D , 2008, vol. 77, no. 09, p.
092001
DOI : 10.1103/PhysRevD.77.092001
Available at:
http://archive-ouverte.unige.ch/unige:38496
Disclaimer: layout of this document may differ from the published version.
Two-particle momentum correlations in jets produced in p p collisions at ffiffiffi p s
¼ 1:96 TeV
T. Aaltonen,23J. Adelman,13T. Akimoto,54M. G. Albrow,17B. A´ lvarez Gonza´lez,11S. Amerio,42D. Amidei,34 A. Anastassov,51A. Annovi,19J. Antos,14M. Aoki,24G. Apollinari,17A. Apresyan,47T. Arisawa,56A. Artikov,15 W. Ashmanskas,17A. Attal,3A. Aurisano,52F. Azfar,41P. Azzi-Bacchetta,42P. Azzurri,45N. Bacchetta,42W. Badgett,17
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K. Yorita,13T. Yoshida,40G. B. Yu,48I. Yu,27S. S. Yu,17J. C. Yun,17L. Zanello,50A. Zanetti,53I. Zaw,22X. Zhang,24 Y. Zheng,8,band S. Zucchelli5
(CDF Collaboration)
1Institute of Physics, Academia Sinica, Taipei, Taiwan 11529, Republic of China
2Argonne National Laboratory, Argonne, Illinois 60439
3Institut de Fisica d’Altes Energies, Universitat Autonoma de Barcelona, E-08193, Bellaterra (Barcelona), Spain
4Baylor University, Waco, Texas 76798
5Istituto Nazionale di Fisica Nucleare, University of Bologna, I-40127 Bologna, Italy
6Brandeis University, Waltham, Massachusetts 02254
7University of California, Davis, Davis, California 95616
8University of California, Los Angeles, Los Angeles, California 90024
9University of California, San Diego, La Jolla, California 92093
10University of California, Santa Barbara, Santa Barbara, California 93106
11Instituto de Fisica de Cantabria, CSIC-University of Cantabria, 39005 Santander, Spain
12Carnegie Mellon University, Pittsburgh, Pennsylvania 15213
13Enrico Fermi Institute, University of Chicago, Chicago, Illinois 60637
14Comenius University, 842 48 Bratislava, Slovakia; Institute of Experimental Physics, 040 01 Kosice, Slovakia
15Joint Institute for Nuclear Research, RU-141980 Dubna, Russia
16Duke University, Durham, North Carolina 27708
17Fermi National Accelerator Laboratory, Batavia, Illinois 60510
18University of Florida, Gainesville, Florida 32611
19Laboratori Nazionali di Frascati, Istituto Nazionale di Fisica Nucleare, I-00044 Frascati, Italy
20University of Geneva, CH-1211 Geneva 4, Switzerland
21Glasgow University, Glasgow G12 8QQ, United Kingdom
22Harvard University, Cambridge, Massachusetts 02138
23Division of High Energy Physics, Department of Physics, University of Helsinki and Helsinki Institute of Physics, FIN-00014, Helsinki, Finland
24University of Illinois, Urbana, Illinois 61801
25The Johns Hopkins University, Baltimore, Maryland 21218
26Institut fu¨r Experimentelle Kernphysik, Universita¨t Karlsruhe, 76128 Karlsruhe, Germany
27Center for High Energy Physics: Kyungpook National University, Daegu 702-701, Korea;
Seoul National University, Seoul 151-742, Korea;
Sungkyunkwan University, Suwon 440-746, Korea;
Korea Institute of Science and Technology Information, Daejeon, 305-806, Korea;
Chonnam National University, Gwangju, 500-757, Korea
28Ernest Orlando Lawrence Berkeley National Laboratory, Berkeley, California 94720
29University of Liverpool, Liverpool L69 7ZE, United Kingdom
30University College London, London WC1E 6BT, United Kingdom
31Centro de Investigaciones Energeticas, Medioambientales y Tecnologicas, E-28040 Madrid, Spain
32Massachusetts Institute of Technology, Cambridge, Massachusetts 02139
33Institute of Particle Physics: McGill University, Montre´al, Canada H3A 2T8;
and University of Toronto, Toronto, Canada M5S 1A7
34University of Michigan, Ann Arbor, Michigan 48109
35Michigan State University, East Lansing, Michigan 48824
36University of New Mexico, Albuquerque, New Mexico 87131
37Northwestern University, Evanston, Illinois 60208
38The Ohio State University, Columbus, Ohio 43210
39Okayama University, Okayama 700-8530, Japan
40Osaka City University, Osaka 588, Japan
41University of Oxford, Oxford OX1 3RH, United Kingdom
42University of Padova, Istituto Nazionale di Fisica Nucleare, Sezione di Padova-Trento, I-35131 Padova, Italy
43LPNHE, Universite Pierre et Marie Curie/ IN2P3-CNRS, UMR7585, Paris, F-75252 France
44University of Pennsylvania, Philadelphia, Pennsylvania 19104
45Istituto Nazionale di Fisica Nucleare Pisa, Universities of Pisa, Siena and Scuola Normale Superiore, I-56127 Pisa, Italy
46University of Pittsburgh, Pittsburgh, Pennsylvania 15260
47Purdue University, West Lafayette, Indiana 47907
48University of Rochester, Rochester, New York 14627
49The Rockefeller University, New York, New York 10021
50Istituto Nazionale di Fisica Nucleare, Sezione di Roma 1, University of Rome ‘‘La Sapienza’’, I-00185 Roma, Italy
51Rutgers University, Piscataway, New Jersey 08855
52Texas A&M University, College Station, Texas 77843
53Istituto Nazionale di Fisica Nucleare, University of Trieste/Udine, Italy
54University of Tsukuba, Tsukuba, Ibaraki 305, Japan
55Tufts University, Medford, Massachusetts 02155
56Waseda University, Tokyo 169, Japan
57Wayne State University, Detroit, Michigan 48201
58University of Wisconsin, Madison, Wisconsin 53706
59Yale University, New Haven, Connecticut 06520 (Received 22 February 2008; published 16 May 2008)
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We present the first measurement of two-particle momentum correlations in jets produced in pp collisions at ffiffiffi
ps
¼1:96 TeV. Results are obtained for charged particles within a restricted cone with an opening angle of 0.5 radians around the jet axis and for events with dijet masses between 66 and 563 GeV=c2. A comparison of the experimental data to theoretical predictions obtained for partons within the framework of resummed perturbative QCD in the next-to-leading log approximation shows that the parton momentum correlations survive the hadronization stage of jet fragmentation, giving further support to the hypothesis of local parton-hadron duality. The extracted value of the next-to-leading-log- approximation parton shower cutoff scaleQeff set equal toQCDis found to beð1:4þ0:90:7Þ 100 MeV. DOI:10.1103/PhysRevD.77.092001 PACS numbers: 13.87.a, 12.38.Qk
I. INTRODUCTION
The goal of this analysis is to measure the two-particle momentum correlation in jets, study its dependence on jet energy, and compare the results to analytical predictions of the next-to-leading log approximation (NLLA) [1].
The evolution of jets is driven by the emission of gluons with very small transverse momenta with respect to the jet axis, i.e. less than 1 GeV=c. The theoretical predictions, which are compared with the results of this measurement, are based on NLLA calculations supplemented with the hypothesis of local parton-hadron duality (LPHD) [2].
NLLA provides an analytical description of parton shower formation, while LPHD states that the hadronization pro- cess takes place locally and, therefore, properties of par- tons and hadrons are closely related. Detailed studies of jet fragmentation allow one to better understand the relative roles of perturbative parton showering and nonperturbative hadronization in shaping the main jet characteristics. Past experimental studies of inclusive distributions of particles in jets ineþe[3] andpp[4,5] collisions have shown good agreement with theoretical predictions, suggesting that the perturbative QCD (pQCD) stage must dominate jet forma- tion, and the role of the nonperturbative stage is reduced to converting final partons into hadrons without significantly affecting their multiplicities and momenta. This paper addresses the question of whether more subtle effects, such as momentum correlation, also survive hadronization.
The predictions for the parton momentum correlations at the level of NLLA precision were first obtained by C. P.
Fong and B. R. Webber in [6] and recently recalculated in the modified leading log approximation (MLLA) frame- work by R. Perez-Ramos [7]. These pQCD-driven corre- lations extend over a large range of parton momenta differences and should not be confused with phenomeno- logical Bose-Einstein correlations [8] present only for parton momenta differences up to 200 MeV.
Until now, the two-particle momentum correlations were studied only by the OPAL Collaboration in eþe collisions at a center-of-mass energy of 91 GeV [9].
Charged particles in the full experimentally accessible solid angle were used in the OPAL analysis. This made it possible for OPAL to ignore some effects of jet reconstruc- tion, but the correlations were measured over a larger cone radius than can be reliably treated theoretically. Strictly
speaking, the theory describes parton shower development only within a small opening anglecaround the jet axis, so thattancc. The OPAL measured distributions showed a pattern in qualitative agreement with theoretical predic- tions, but the values of the parton shower cutoff Qeff [1]
extracted from the fit of the correlation distributions were inconsistent with theQeff extracted from fits of the inclu- sive momentum distributions [10].
In this paper, we report a measurement of the two- particle momentum correlation for charged particles in events with dijet invariant masses in the range 66–563 GeV=c2. Momentum correlation distributions are measured for charged particles in restricted cones with an opening angle of c¼0:5 radians around the jet axis.
Events were produced at the Tevatron collider inpp colli- sions at a center-of-mass energy of 1.96 TeV and were recorded by the CDF II detector. The total integrated luminosity is385 pb1.
The data sample consists of events with an expected mixture of quark and gluon jets. In order to compare experimental results with theoretical predictions, the analysis is carried out in the center-of-mass system of the two jets. The data are divided into seven bins according to the value of dijet invariant mass, which allows us to explore the dependence of correlation parameters on energy.
The data are fit to NLLA analytical functions and the value of the parton shower cutoff Qeff is extracted. The correlations observed in data are compared to Monte Carlo predictions by thePYTHIAtune A [11,12] andHERWIG6.5 [13] event generators.
II. THEORY
A. Next-to-leading log approximation
NLLA allows a perturbative calculation of the parton shower by keeping all terms of order nsln2nðEjetÞ and nsln2n1ðEjetÞ at all orders n of perturbation theory. In these terms s is the strong coupling constant andEjet is the jet energy. Most of the particles in jets have kT<
1 GeV=c[5], wherekT is the transverse momentum with respect to the jet axis. Therefore, in order to successfully describe jet fragmentation, a theoretical model must be able to handle parton emissions at such low transverse momenta scales.
In NLLA the requirement that partonkT > Qcutoff, for a sufficiently high cutoff scale Qcutoff (typically a few GeV=c), ensures that only partons in the perturbative region are included in the calculation. After the resumma- tion the value of the parameterQcutoffcan be lowered to the value ofQCD. Lowering the parameter Qcutoff is equiva- lent to including softer partons in the description of the model. SettingQcutoffto its lowest value,QCD, maximizes the range of applicability of the model. The phenomeno- logical scale replacing the two initial parameters Qcutoff and QCD is conventionally called Qeff. In theoretical calculations final expressions for the observables of inter- est are usually functions of ¼lnðQ=QeffÞ, where Q¼ Ejetcis the so-called jet hardness. These final expressions can be expanded in powers of . The Fong-Webber ap- proach [6] keeps only terms that are fully controlled within the precision of the calculation, i.e. neglects all terms of order nsln2n2ðEjetÞ and higher. The Perez-Ramos ap- proach [7] partially includes higher-order terms.
The inclusive momentum distribution function of par- tons in jetsDðÞ ¼dNd in NLLA is defined in terms of the variable ¼lnð1xÞwhere x¼Ep
jet andpis the parton mo- mentum. This distribution is predicted to have a distorted Gaussian shape [14]:
dN
d ¼ N ffiffiffiffiffiffiffi
2 p exp
1
8l1 2s1
4ð2þlÞ2þ1 6s3 þ 1
24l4
; (1)
where¼0 and0is the position of the maximum of the distribution. The coefficients , s, and l are the width, skewness, and kurtosis of the inclusive momentum spectrum. These coefficients are calculated to next-to- leading order and depend on Qeff. Overall, the function has three parameters to be determined experimentally: the normalizationN, Qeff, and an unknown higher-order cor- rection term Oð1Þ [6] in the calculation of 0 ¼0:5þ a ffiffiffi
p
þOð1Þ, where a is a constant that depends on the number of colors and the number of effectively massless quarks. The unknown term Oð1Þ is expected to be inde- pendent of. The predicted dependence of the inclusive momentum distribution on jet hardness is shown in Fig.1.
The two-parton momentum correlation function Rð1; 2Þ is defined to be the ratio of the two- and one- parton momentum distribution functions:
Rð1; 2Þ ¼ Dð1; 2Þ
Dð1ÞDð2Þ; (2) where Dð1; 2Þ ¼dd2N
1d2. The momentum distributions are normalized as follows:R
DðÞd¼ hni, wherehni is the average multiplicity of partons in a jet, and RDð1; 2Þd1d2¼ hnðn1Þi for all pairs of partons in a jet. The average multiplicity of partons hni is a function of the dijet massMjjand the size of the opening
anglec. Forc ¼0:5,hnivaries from6to12forMjj in the range80–600 GeV=c2 [4].
The Fong-Webber approximation of Eq. (2) for the two- parton momentum correlation function [6] can be written as follows:
Rð1;2Þ ¼r0þr1ð1þ2Þ þr2ð12Þ2; (3) where ¼0, and the parameters r0, r1, and r2 define the strength of the correlation and depend on the variable ¼lnðQ=QeffÞ. Equation (3) is valid only for partons with around the peak of the inclusive parton momentum distribution, in the range 1. The pa- rametersr0,r1, andr2 are calculated separately for quark and gluon jets from an expansion in powers of1= ffiffiffi
p using the assumption that the number of effectively massless quarks Nf is 3. Keeping only terms controlled by theory, the parameters are
rq0 ¼1:750:64ffiffiffi
p ; rq1 ¼ 1:6
3=2; rq2 ¼ 2:25 2 ;
(4) rg0 ¼1:330:28ffiffiffi
p ; rg1 ¼ 0:7
3=2; rg2 ¼ 1:0 2 ; (5) whereqandgsuperscripts denote the correlation parame- ters for partons in quark jets and gluon jets, respectively.
The theoretical prediction of the shape of the two-parton momentum correlation distribution function is shown in Fig.2. Along the central diagonal1 ¼ 2, the shape of the two-parton momentum correlation is parabolic with a maximum at 1 ¼2. Along the central diagonal
ξ
0 1 2 3 4 5 6 7 8
ξdN/d
0 0.5 1 1.5 2 2.5 3 3.5 4 4.5
c=0.5 θ Cone Q=19 GeV
Q=50 GeV Q=119 GeV
FIG. 1. NLLA inclusive parton momentum distributions for Q¼Ejetc¼19, 50, and 120 GeV and Qeff ¼230 MeV cal- culated according to [14].
1 ¼2, the shape is linear and increasing toward larger values of , i.e. lower momentum partons.
Therefore, the obvious features of the prediction are (1) the correlation should be stronger for partons with equal momenta 1 ¼2, and (2) the strength of this effect should increase for lower momentum partons.
B. Normalization
The correlation function from Eq. (2) includes two effects: (1) multiplicity fluctuations of partons in a jet and (2) actual momentum correlations. In this analysis, we measure pure momentum correlations. This can be achieved by introducing one- and two-parton momentum distributions normalized to unity:
D0ðÞ ¼DðÞ
hni ; Z
D0ðÞd¼1; (6)
D0ð1; 2Þ ¼ Dð1; 2Þ hnðn1Þi; Z
D0ð1; 2Þd1d2¼1: (7) Then, the correlation function can be defined as Cð1;2Þ ¼ D0ð1; 2Þ
D0ð1ÞD0ð2Þ¼ hni2
hnðn1ÞiRð1;2Þ
¼ 1
FðÞRð1;2Þ; (8) whereFðÞ ¼hnðn1Þihni2 is the second binomial moment. The explicit dependence of the binomial moments on the en- ergy scale for quark and gluon jets is taken from theory [15]:
FqðÞ ¼1:751:29ffiffiffi
p ; FgðÞ ¼1:330:55ffiffiffi p : (9)
C. Quark and gluon jets
In theory, correlation functions are calculated for quark and gluon jets separately and are denoted by DqðÞ and DgðÞ, respectively. Since dijet events at the Tevatron consist of both quark and gluon jets, in order to compare data to theory, we rewrite the formula for the parton momentum distributions as follows:
DðÞ ¼fgDgðÞ þ ð1fgÞDqðÞ; (10) Dð1; 2Þ ¼fgDgð1; 2Þ þ ð1fgÞDqð1; 2Þ; (11) where fg is a fraction of gluon jets in the sample. After simple algebraic transformations, it can be shown that the momentum correlation Eq. (8) is reduced to the following:
Cð1;2Þ ¼c0þc1ð1þ2Þ þc2ð12Þ2; (12) where thecicoefficients (i¼0, 1, 2) are
ci¼ fgr2
fgr2Fgþ ð1fgÞFqrgi þ 1fg
fgr2Fgþ ð1fgÞFqrqi; (13) where r¼hnhngqii is the ratio of average multiplicities of partons in gluon and quark jets. The value of r enters in the derivation of Eqs. (4) and (5) [6], Eq. (9) [15], and Eq. (13). In NLLA this ratio is equal to9=4. Values ofrby thePYTHIA6.115 andHERWIG5.6 Monte Carlo generators are given in [16].
D. Local parton-hadron duality
LPHD is a hadronization conjecture that suggests that the properties of hadrons and partons are closely related. In the simplest interpretation of LPHD, each parton at the end of the pQCD shower development picks up a color- matching partner from the vacuum sea and forms a hadron.
Within LPHD, the momentum distributions of hadrons are related to those of partons via an energy-independent constantKLPHD:
dNhadrons
d ¼KLPHDdNpartons
d : (14) Past studies of inclusive particle distributions at eþe experiments [3] and CDF [4,5] have given strong support to the LPHD hypothesis. In this analysis, we extend the LPHD test by examining whether the two-particle momen- tum correlations predicted in the pQCD framework also survive the hadronization. Note that in the two-particle momentum correlation given by Eq. (2), KLPHD simply cancels, suggesting that the correlation distributions for hadrons and partons are expected to be the same.
ξ1
∆
-1 -0.5 0 0.5 1
2ξ∆
-1 -0.5 0 0.5 1
1.1 1.15 1.2 1.25 1.3
ξ2
=∆ ξ1
∆
ξ2
=-∆ ξ1
∆
FIG. 2. The NLLA parton momentum correlation function calculated for a gluon jet, Q¼50 GeV, and Qeff ¼ 230 MeVaccording to [6].
III. CDF II DETECTOR
Data used in this analysis were recorded with the CDF II detector. The detector was designed for precision measure- ments of the energy, momentum, and position of particles produced in proton-antiproton collisions. This section pro- vides a brief overview of the components relevant to our analysis. A detailed description of the entire detector can be found elsewhere [17].
CDF II uses a cylindrical coordinate system with the positivezdirection selected along the proton beam direc- tion and the azimuthal anglemeasured around the beam axis. The polar angle is measured with respect to the positivezdirection and the pseudorapidity is defined as
¼ ln½tanð2Þ.
The CDF II tracking system is placed inside a 1.4 T solenoidal magnet. A layer 00 single-sided silicon micro- strip detector is mounted directly on the beam pipe, at an inner radius of 1.15 cm and an outer radius of 2.1 cm. A five-layer silicon microstrip detector (SVX II) is closest to the beam line, and is situated at a radial distance of 2.5 to 11 cm from the beam. The SVX II consists of three separate barrel modules with a combined length of 96 cm. Three of the five layers combine ar- measure- ment with az-coordinate measurement, while the remain- ing two layers combiner-with a small stereo angle of 1.2. Three additional intermediate silicon layers (ISL) are positioned between 19 and 30 cm. The SVX II is sur- rounded by the central outer tracker (COT), an open-cell drift chamber providing up to 96 measurements of a charged particle track over the radial region from 40 to 137 cm. The 96 COT measurements come from 8 super- layers of 12 sense wires each. The superlayers alternate between axial and 3 stereo. The pseudorapidity region covered by the COT is j j<1:0. The momentum of a charged particle is determined by the curvature of its trajectory in the magnetic field.
The CDF II tracking system is surrounded by calorim- eters used to measure the energy of charged and neutral particles. In the central region the central electromagnetic (CEM), central hadronic (CHA), and wall hadronic calo- rimeters are made of lead (electromagnetic) and iron (had- ronic) layers interspersed with scintillator. The pseudo- rapidity region covered by these calorimeters isj j<1:3. The segmentation of the central calorimeters is 15 in and 0.1 units in . The measured energy resolutions for the CEM and CHA are ðEÞ=E¼13:5%= ffiffiffiffiffiffi
ET
p 2% and
ðEÞ=E¼75%= ffiffiffiffiffiffi
ET
p 3%, respectively. Here ET¼ Esinis transverse energy of an incident particle (electron for CEM and pion for CHA) and energies are measured in GeV.
IV. EVENT SELECTION A. Triggers
Events were collected using a single-tower trigger [18]
with a transverse energyETthreshold of 5 GeV (ST05) and
with single jet triggers withETthresholds of 20 (J020), 50 (J050), 70 (J070), and 100 (J100) GeV. Each of the jet triggers had a different sampling rate so as not to saturate the available trigger bandwidth.
B. Jet reconstruction algorithm
Jets are reconstructed based on the calorimeter informa- tion using a cone algorithm [19]. The algorithm starts with the highest transverse energy tower and forms preclusters from an unbroken chain of continuous seed towers with transverse energy above 1 GeV within a window of77 towers centered at the originating seed tower. If a seed tower is outside this window, it is used to form a new precluster. The coordinates of each precluster are the ET-weighted sums of and of the seed towers within this precluster. In the next step, all towers with ET>
0:1 GeV within R¼ ffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffi ðÞ2þ ð Þ2
p ¼1:0 of the pre-
cluster are merged into a cluster, and itsð ; Þcoordinates are recalculated. This procedure of calculating cluster coordinates is iterated until a stable set of clusters is obtained. A cluster is stable when the tower list is un- changed from one iteration to the next. If the clusters have some finite overlap, then an overlap fraction is com- puted as the sum of theET of the common towers divided by theET of the smaller cluster. If the fraction is above a cutoff value equal to 0.75, then the two clusters are com- bined. If the fraction is less than the cutoff, the shared towers are assigned to the closest cluster. The raw energy of a jet is the sum of the energies of the towers belonging to the corresponding cluster. Corrections are applied to the raw energy to compensate for the nonlinearity and nonun- iformity of the energy response of the calorimeter, the energy deposited inside the jet cone from sources other than the leading parton, and the leading parton energy deposited outside the jet cone. A detailed description of this procedure can be found in [20].
C. Offline selection
Cosmic ray events are rejected by applying a cutoff on the missing transverse energyE6 Tsignificance [21], defined as E6 T= ffiffiffiffiffiffiffiffiffiffi
ET
p , where ET ¼iEiT is the total transverse energy of the event, as measured using calorimeter towers withEiTabove 100 MeV. The thresholds are3:0 GeV1=2for data collected using a single-tower trigger withETthresh- old of 5 GeV, and 3.5, 5.0, 6.0, and 7:0 GeV1=2 for data collected using jet triggers with thresholds of 20, 50, 70, and 100 GeV, respectively.
To ensure fully efficient vertex and track reconstruction, we require only one vertex in the event withjzj<60 cm. To ensure robust and high efficiency track reconstruction and applicability of the background removal technique (see Sec. V B), only events with both leading jets in the central region (j j<0:9) are selected. To reject events with poorly measured jets, we require the two leading jets to
be well balanced inET: k?=ðE1TþE2TÞ<2k?. Here E1T and E2T are the transverse energies of the first and the second leading jets, respectively, andk? is
k?¼ ffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffi k2k2jj q
; (15)
kjj ¼ ðE1TþE2TÞ cosð =2Þ; (16) wherek~is a vector sum of momenta of the two leading jets, is the angle between the two leading jets, andk?is the resolution of k?. The definitions of k,~ k?, and kjj are illustrated in Fig. 3. The component k? is known to be sensitive to jet energy mismeasurements, whilekjj is more sensitive to hard gluon radiation.
In events with high energy jets, a single particle emerg- ing from a jet at a sufficiently large angle with respect to the jet axis can be mistakenly identified as a separate jet. A jet can also be produced from the underlying event.
Therefore, rejection of all events with more than two jets can introduce possible biases. We allow up to two extra jets, but their energy is required to be small: EextraT <
5:5 GeVþ0:065ðE1TþE2TÞ, whereEextraT is the transverse energy of an extra jet.
After application of the event selection cuts, the final sample consists of approximately 250 000 events and is further divided into seven bins according to the dijet mass as measured by the calorimeters and defined as
Mjj¼ ffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffiffi ðE1þE2Þ2=c4 ðP~1þP~2Þ2=c2 q
; (17) where E andP~ are the energies and momenta of the two leading jets, respectively.
The mass bin boundaries, average invariant masshMjji, and number of events in each bin are given in TableI. The bin width is selected to be 3Mjj, where Mjj is the calorimeter resolution for the dijet mass determination,
Mjj
Mjj 10%–15%. Events with dijet invariant mass below 66 GeV=c2are not used in the measurement because of the lower trigger efficiency.
D. Systematic uncertainties associated with the event selection
The sensitivity of the two-particle momentum correla- tion parametersc0,c1, andc2to various uncertainties in the event selection procedure is evaluated as follows. For each source of systematic uncertainty the so-called ‘‘default’’
and ‘‘deviated’’ two-particle momentum correlation distri- butions are obtained. The default distribution is produced using the standard selection requirements described in this article. Then, the deviated distribution is obtained by vary- ing all relevant parameters according to the estimated systematic uncertainty (one source of uncertainty at a time). For each bin in correlation Cð1;2Þ, a scale factor is calculated by taking the bin-by-bin ratio of the deviated and default distributions:
¼Cð1;2Þdeviated Cð1;2Þdefault
: (18)
The difference between correlation distributions in the data with and without this bin-by-bin scale factor is taken as a measure of the systematic uncertainty:
Cð1;2ÞData¼ jð1Þ Cð1;2ÞDataj: (19)
Jet1
Jet2 k|| k
kT ψ
FIG. 3. Definition of variables for the jet balance requirement.
The plane perpendicular to the beam line is shown. The vector k~ represents a vector sum of the two leading jets’ momenta. The kjjand k?components of k~are parallel and perpendicular to the bisector of the two jets, respectively.
TABLE I. Dijet mass bin boundaries, average dijet invariant mass hMjji, average Ejet-weighted jet hardness Q, and number of events in each bin after the event selection requirements Nev.
Bin Trigger Low edge (GeV=c2) High edge (GeV=c2) hMjji (GeV=c2) Q(GeV) Nev
1 ST05 66 95 76 19 15 229
2 J020 95 132 108 27 77 246
3 J020 132 180 149 37 17 682
4 J050 180 243 202 50 80 608
5 J050 243 323 272 68 18 528
6 J070 323 428 361 90 12 000
7 J100 428 563 475 119 19 150
Further in this section, we discuss sources of systematic uncertainties at the level of the event selection; their con- tributions to the values of c0, c1, and c2 are given in TableII.
In each trigger sample only the events with trigger efficiency higher than 99% are used. To check that trigger effects do not bias the measurement, we verify the con- tinuity of the distributions of particle multiplicity in a jet in the transition between adjacent dijet trigger samples. No detectable offsets are observed.
To evaluate the uncertainty due to the value of the parameterRof the jet reconstruction algorithm, we com- pare the results of the measurement using three different values ofR (0.4, 0.7, 1.0). This effect proved to be small compared to the other sources of systematic uncertainty.
We require only one vertex in the event, which greatly reduces the contribution of multiple proton-antiproton in- teractions in the same bunch crossing. However, in some cases two vertices can be very close to each other and be reconstructed as a single vertex. This can become signifi- cant at high instantaneous luminosity. To evaluate the uncertainty due to this effect, we divide each dijet mass bin into smaller bins based on the instantaneous luminos- ity. Momentum correlation distributions are compared in these smaller samples and the difference is taken as a measure of the systematic uncertainty.
To evaluate the uncertainty due to the jet energy correc- tions, we use parametrizations in which the jet energy scale is shifted by plus or minus 1 standard deviation [20]. We then reclassify the events according to their dijet mass. The difference between the default and deviated distribution is assigned to be the systematic uncertainty.
We use Monte Carlo dijet samples produced byPYTHIA
tune A to study systematic uncertainties associated with the jet balance requirement, the number of allowed extra jets, and their energy. The default two-particle momentum correlation distribution is compared to the deviated one.
The deviated distribution has no requirements imposed on the jet balance or on the extra jet number and extra jet energy.
Monte Carlo simulations are used to evaluate the sys- tematic uncertainty due to mismeasurement of the jet
direction. Two-particle momentum correlations are com- pared for two cases. In one case particles are counted in a restricted cone around the jet direction as determined by the detector response in the simulation. In the second case the direction of primary partons from the hard scattering as given byPYTHIAtune A is used for the cone axis.
V. TRACK SELECTION, CORRECTIONS, SYSTEMATIC UNCERTAINTIES
Measurements described below are performed in the dijet center-of-mass frame. For Lorentz boosts all particles are treated as pions. Experimentally we define the variable as¼lnð1=xÞ ¼lnpEjet
track, whereEjet is the jet energy as
measured by the calorimeters and ptrack is the track mo- mentum as measured by the tracking system. The correla- tion distributions are measured for all track pairs that pass track quality requirements and lie within a restricted cone of opening anglec¼0:5radians relative to the jet axis.
The peak position of the inclusive momentum distribution 0 is constant for a given jet hardnessQ and is obtained from the data. The measurements are corrected for various backgrounds both correlated and uncorrelated with jet direction.
A. Track quality requirements
Several selection requirements are applied to ensure that the tracks in the measurement originate at the primary vertex and are not produced by cosmic rays, multiplepp interactions within the same bunch crossing, conver- sions,K0 anddecays, or other types of backgrounds.
In our analysis we require full three-dimensional track reconstruction. The description of CDF II track reconstruc- tion can be found in [22,23]. Poorly reconstructed and spurious tracks are removed by requiring a good track fitting parameter 2COT<6:0. Charged particles are re- quired to have transverse momentumpT>0:3 GeV=c.
The parameterzis defined as the difference between the z position of the track at the point of its closest approach to the beam line and thezposition of the primary vertex. This parameter is used to remove tracks not orig- inating at the primary interaction by requiring jzj<5 TABLE II. Summary of the systematic uncertainties of the correlation parameters c0, c1, and
c2 for the dijet mass bin with Q¼50 GeV.
Origin of systematic uncertainty c0 c1 c2
Luminosity dependence 0.001 0.004 0.002
Jet energy scale 0.001 0.001 0.001
Balance and extra jet cuts 0.006 0.001 0.003
Mismeasurement of jet direction 0.006 0.008 0.007
Track quality cuts 0.014 0.008 0.006
Underlying event background 0.001 0.004 0.001
Tracking inefficiency 0.011 0.001 0.002
Neutral particles 0.002 0.002 0.001
