Quantifying jet transport properties via large $p_T$ hadron production

Nuclear modification factor $R_{AA}$ for large $p_T$ single hadron is studied in a next-to-leading order (NLO) perturbative QCD (pQCD) parton model with medium-modified fragmentation functions (mFFs) due to jet quenching in high-energy heavy-ion collisions. The energy loss of the hard partons in the QGP is incorporated in the mFFs which utilize two most important parameters to characterize the transport properties of the hard parton jets: the jet transport parameter $\hat q_{0}$ and the mean free path $\lambda_{0}$, both at the initial time $\tau_0$. A phenomenological study of the experimental data for $R_{AA}(p_{T})$ is performed to constrain the two parameters with simultaneous $\chi^2/{\rm d.o.f}$ fits to RHIC as well as LHC data. We obtain for energetic quarks $\hat q_{0}\approx 1.1 \pm 0.2$ GeV$^2$/fm and $\lambda_{0}\approx 0.4 \pm 0.03$ fm in central $Au+Au$ collisions at $\sqrt{s_{NN}}=200$ GeV, while $\hat q_{0}\approx 1.7 \pm 0.3$ GeV$^2$/fm, and $\lambda_{0}\approx 0.5 \pm 0.05$ fm in central $Pb+Pb$ collisions at $\sqrt{s_{NN}}=2.76$ TeV. Numerical analysis shows that the best fit favors a multiple scattering picture for the energetic jets propagating through the bulk medium, with a moderate averaged number of gluon emissions. Based on the best constraints for $\lambda_{0}$ and $\tau_0$, the estimated value for the mean-squared transverse momentum broadening is moderate which implies that the hard jets go through the medium with small reflection.


I. INTRODUCTION
A strongly coupled quark gluon plasma (sQGP) consisting of deconfined quarks and gluons may have been created in the central region of high-energy nuclear collisions at the BNL Relativistic Heavy Ion Collider (RHIC) and the CERN Large Hadron Collider (LHC). One important evidence for the formation of sQGP from the experiment results are the jet quenching phenomena [1,2] that include the strong suppression of single hadron spectra [3][4][5][6], back-to-back dihadron [7,8] and photontriggered hadron [9,10] as well as jet productions [11,12] with large transverse momentum in central A + A collisions as compared to p + p collisions. These observed jet quenching patterns in heavy-ion collisions at RHIC/LHC can be described well by different theoretical models [13][14][15][16][17][18][19][20][21][22][23][24] that incorporate parton energy loss induced by multiple parton scattering and gluon bremsstrahlung as it propagates through the dense matter.
A widely used parameter controlling the parton energy loss is the jet transport parameterq [25], or the mean-squared transverse momentum broadening per unit length for a jet in a strong interacting medium, which is also related to the gluon distribution density of the medium [25,26] and therefore characterizes the medium property as probed by an energetic jet. To estimate the jet transport parameterq intense theoretical studies have been made, such as with the weakly-coupled QCD [27][28][29], the strong-coupled AdS/CFT [30,31], and the lattice calculations [32,33]. Recently, a phenomenological investigation had been carried out to extract the initial value of jet transport coefficientq 0 at initial time τ 0 , which givesq 0 ≈ 1.2 ± 0.3 GeV 2 /fm in Au+Au collisions at √ s N N = 200 GeV andq 0 ≈ 1.9±0.7 GeV 2 /fm in Pb+Pb collisions at √ s N N = 2.76 TeV for a given quark with initial energy of 10 GeV [34].
In this paper we will extract the initial jet transport parameterq 0 and the initial mean free path λ 0 at initial time τ 0 on the bulk medium evolution by comparing the experimental data at RHIC/LHC with numerical simulations of of single hadron yields with large p T in a next-to-leading order (NLO) pQCD parton model, where the EPS09 parametrization set of NLO nuclear parton distribution functions (nPDFs) has been used to take into account of possible initial-state cold nuclear matter effects, and a phenomenological model [17,19] for medium-modified fragmentation functions calculated in leading-order (LO) at twist-4 in the high-twist approach of jet quenching [35][36][37] has been utilized to incorporate parton energy loss. The evolution of bulk medium used in the study for parton propagation was given by a 3 + 1 dimensional ideal hydrodynamic model [38,39] which is constrained by experimental data on hadron spectra. From calculations with the two independent inputs for the parameters and simultaneous χ 2 /d.o.f fits to the RHIC and the LHC data, we obtain that for energetic quarksq 0 ≈ 1.1 ± 0.2 GeV 2 /fm and λ 0 ≈ 0.4 ± 0.03 fm in central Au + Au collisions at √ s N N = 200 GeV, whileq 0 ≈ 1.7 ± 0.3 GeV 2 /fm, and λ 0 ≈ 0.5 ± 0.05 fm in central P b + P b collisions at √ s N N = 2.76 TeV. This simultaneous and separate constraint of the two initial values should give a precise and quantitative description for jet quenching to probe the medium properties. For a parton jet propagating through the bulk medium, the average transverse momentum broadening squared q 2 T depends on the transport parameter as well as the mean free path, q 2 T =qλ. Our numerical results show that the mean transverse momentum broadening squared of energetic partons for one scattering at initial time τ 0 in the center of the fireball at LHC is about 2 times of that at RHIC. The rest of the paper is organized as follows. We first give a brief overview of the NLO pQCD parton model for single inclusive hadron spectra and a phenomenological model for medium-modified fragmentation functions in Sec. II. Then the numerical calculations for phenomenological studies of the experimental data on single hadron suppression and extraction of the jet transport parameter and the mean free path are carried out in Sec . III. We present some discussions in Sec. IV and finally summarize our study in Sec. V.

II. NLO PQCD PARTON MODEL AND MODIFIED FRAGMENTATION FUNCTIONS
We will utilize the pQCD parton model at NLO for the initial jet production spectra which has been applied to large p T hadron production in high energy hadronhadron reactions with great successes [40]. In the model the differential cross section of hadron yields has been expressed as a convolution of NLO parton-parton scattering cross sections, parton distribution functions (PDFs) in nucleons and parton fragmentation functions (FFs), where dσ(ab → cd)/dt denotes the leading-order (LO) elementary parton scattering cross sections at α 2 s . The NLO contributions in O(α 3 s ) involve both 2 → 3 tree level processes and one loop virtual corrections to 2 → 2 tree processes. Processes at 2 → 3 tree level inlcude qq → qqg, qq → qqg, qq → ggg, qg → qgg, qg → qqq, gg → qqg, gg → ggg, etc, which include soft and collinear contributions. A standard M S renormalization scheme is applied to control ultraviolet divergence in one loop virtual corrections to 2 → 2 tree processes. More detailed discussions on calculations at NLO could be found in [41]. In this paper the numerical calculations are carried out with a NLO Monte Carlo program [40] where two cut-off parameters, δ s and δ c , are employed to isolate the collinear and soft divergences in the squared matrix elements of the 2 → 3 processes. The regions with the divergences are integrated over in n-dimension phase space and the results are added with the squared matrix elements of the 2 → 2 processes. This gives a set of twobody and three-body weights depending on δ s and δ c . But the dependence will be eliminated after the weights are combined in the calculation of physical observables, and the final numerical results are insensitive to the cutoff parameters [40].
We employ the same factorized form for the inclusive large p T particle production cross section in nucleusnucleus collisions, which can be computed as a convolution of nuclear thickness functions, the nuclear parton distribution functions (nPDFs), elementary partonparton scattering cross sections and effective medium-modified parton fragmentation functions (mFFs) [17,19], at fixed impact parameter b in the transverse plane of the beam direction. In Eq.
(2) the average over the azimuthal angle of the initial fast parton is implicitly implied. The nuclear thickness function t(r) is calculated with the Woods-Saxon distribution function for nucleons in a nucleus and has been normalized by requiring d 2 rt A (r) = A. The nuclear parton distributions per nucleon (nPDFs) f a/A (x a , µ 2 , r) can be parameterized as the production of the parton distributions inside free nucleons f a/N (x, µ 2 ) and the nuclear shadowing factor S a/A (x, µ 2 , r), where Z denotes the charge and A is the mass number of the nucleus. In the numerical simulations we use the CTEQ6M parametrization [42] for nucleon parton distributions f a/N (x, µ 2 ), and EPS09 parametrization of nPDFs [43]. Since the parton-parton scattering cross sections are computed up to NLO, the CTEQ6M parametrization and EPS09 parametrization are both used at NLO. For simplicity, we only use the centralfit set of EPS09 parametrization in following numerical calculations.
An energetic parton jet produced in the hard scattering may suffer multiple scattering with thermal partons in the QGP created in nucleus-nucleus collisions. The jet-medium scattering and medium induced gluon radiation should give rise to new contributions to parton fragmentation functions (FFs) in vacuum and thus leads to medium-modified fragmention functions, which may evolve with the scale Q [14,17,19,46,47], in a similar way like the DGLAP evolution in vacuum. If the parton jet travels a distance L inside the medium with the inelastic scattering mean free path λ, the probability for the jet scattering n times to the medium can be assumed to obey Poisson distribution [44,45]. Therefore, effect of parton energy loss in the dense QCD medium can be calculated in the high-twist approach of jet quenching and the effective medium-modified parton fragmentation functions (mFFs) can be given by [14,17,19,46], is the rescaled momentum fraction of the hadron from the fragmentation of the quenched parton which has the initial transverse momentum p T c and loses energy ∆E c during its propagation inside the hot medium, z ′ g = L/λ p T /∆E c is the rescaled momentum fraction of the hadron from the fragmentation of a radiated gluon with initial energy ∆E c / L λ , and z c = p T /p T c is the momentum fraction for jet fragmentation in vacuum. L λ times scattering will provide L λ gluon emissions, so there is a factor L λ in the fragmentation contribution of emitted gluon in above equation. As shown in Ref. [44], the above mFFs satisfy the momentum sum rule by construction, The weight factor exp(− L λ ) is the probability for those partons escaping the medium without suffering any inelastic scattering, and the weight factor 1 − exp(− L λ ) is the probability for partons encountering at least one inelastic scattering. The rescaled fraction in Eq. (4) is got by energy shifting due to energy loss ∆E c . For a given jet, the energy loss ∆E c and the scattering number L λ both depend on the local medium density in the jet trajectory and characterize the medium properties. This approximative approach for medium-modified fragmentation function reproduces the main effect of mediuminduced radiation [14], and is therefore similar to another approximative approach in references [48,49] where the modified fragmentation function is concluded as a convolution of the vacuum fragmentation function and the probability for a given jet to be quenched to a final jet inside the medium. We also note the difference between our approach and the ones used in references [48,49]. In higher-twist formalism [35][36][37], one considers twist-4 processes of the splitting of a highly virtual parton (µ >> Λ QCD ) in QCD medium and evaluates the contribution of medium-induced gluon radiation, which gives rise to the effectively modified parton fragmentation functions and their corresponding (medium-modified) QCD evolution equations with respect to the hard scale µ. This is different from that in references [48,49] where the medium contribution is computed at the medium scale. Also in references [48,49] a convolution with a Poisson probability for multiple emissions is used for the energy shift to take into account the fluctuation of energy loss.
In a high-twist approach the total energy loss ∆E = ∆E c (E, b, r) is related to the jet transport parameter via, as shown in Ref. [50], in which one can refer for more details. y − denotes a jet place in its trajectory, and is the same as normal time τ used in following calculations. In the above expression, the LPM effect for the induced gluon emission originates from the destructive interference of two kinds of processes, i.e. the soft-hard and hard-hard processes, which become identical to each other and lead to a cancellation of their contributions when the transverse momentum of the radiated gluon is small and the formation time of radiated gluon is rather large [35][36][37]. This is exactly the same as the LPM effect in the double scattering in the GLV opacity expansion formalism [51]. In the case of multiple soft scattering, as discussed in references [25,29,[52][53][54] the LPM effect is caused by similar interferences and plays a dominant role when the coherent emission of a single gluon in a multiple scattering process is considered and leads to a suppression of the energy loss as compared to the additive contribution of n(= L λ ) independent scattering of one gluon radiation.
We emphasize that in our model, the parton matrix elements are calculated at NLO, and EPS nuclear PDFs at NLO are utilized to include the initial-state cold nuclear matter effects, whereas the parton energy loss due to the final-state hot medium effect is given by a LO derivation of parton energy loss resulting from effective medium-modified fragmentation functions in twist-4 at the high-twist expansion approach. Recently several theoretical attempts [27-29, 55, 56] have been made to calculate momentum broadening and parton energy loss due to multiple scattering in medium beyond leading order, which may be incorporated phenomenologically to a complete NLO calculations of particle or jet productions in high-energy nuclear collisions. It is also noticed that recently theoretical investigation of color decoherence has been developed for jets resolving and energy redistributing in the QCD medium [57][58][59].
The jet transport parameter for a gluon is 9/4 times of a quark, which is assumed to be proportional to the local parton density in a dynamical evolving medium and expressed as [20,60,61], for a parton produced at a transverse position r at an initial time τ 0 and traveling along the direction n.q 0 denotes the jet transport parameter at the center of the bulk medium at the initial time τ 0 . ρ g is the gluon density at a given temperature T (τ, r), and in numerical calculations we assume ρ g ∝ (1 − f )T 3 for the medium as an ideal gas. As introduced in Ref. [38,39,60], the fraction f (τ, r) of the hadronic phase at any given time and local position is given by where we consider the mixed phase contribution and neglect the pure hadron phase contribution. During the mixed phase at T = 170 MeV the hadron phase fraction will be f = 0 ∼ 1 while the QGP phase faction will be 1 − f . With the time evolution during the mixed phase the fraction value f will increase from 0 to 1. In the following numerical calculations the time-dependent fraction f is given by simulations of the hydrodynamic model [38,39]. p µ is the four momentum of the jet and u µ is the four flow velocity in the collision frame. The average number of scatterings along the parton propagating path is given by, where λ 0 is the mean free path at the initial time τ 0 , and for a quark jet it is 9/4 times of that for a gluon jet. The parameter λ 0 as well asq 0 will be independently inputted in the following numerical calculations and simultaneously constrained by experiment data. The fragmentation function in vacuum D 0 h/c (z c , µ 2 ) in Eq. (1) and (4) is given by the AKK parametrization [62]. Here we use the NLO AKK FFs parametrization. For inclusive hadron production given by Eq. (1) and (2), there are three independent scales: the renormalization scale µ ren , the factorization scale µ f act and the fragmentation scale µ f rag . We choose µ ren = µ f act = µ f rag = 1.2p T in our numerical analysis for both p+p and A+A collisions.
In the model for the effective medium-modified fragmentation functions (mFFs) disucssed in Sec. III, information on the space-time evolution of the local temperature and flow velocity in the bulk medium along the jet propagation path should be provided. In our simulation we will utilize a (3+1) dimensional ideal hydrodynamic model [38,39] to obtain the space-time evolution of the bulk matter created in central nucleus-nucleus collisions.
With a given space-time profile of the gluon density, one can then utilize the preceding effective mFFs to obtain the high p T hadron spectra. In actual calculations for the spectra or cross section at fixed values of the hadron transverse momentum p T in Eq. (1) and (2), the factorization and renormalization scales are all chosen as µ f = µ R = 1.2 p T . Shown in Fig. 1 (a) are the hadron cross sections in p + p and 0-5% Au + Au collisions at √ s N N = 200 GeV with given parameter valuesq 0 = 1.1 GeV 2 /fm and λ 0 = 0.4 fm, as compared to PHENIX data [63][64][65]. The theoretical cross section for A + A collisions is scaled as . We choose b = 2 fm for 0-5% Au + Au and b = 2.1 fm for 0-5% P b + P b collisions. Shown in Fig. 2 (a) are for 0-5% P b + P b collisions with given parameter valuesq 0 = 1.7 GeV 2 /fm and λ 0 = 0.5 fm, as compared to CMS and ALICE data [5,6]. It is observed that the theoretical results with chosen parameters ofq 0 and λ 0 could describe the experimental data at the RHIC and the LHC very well. Shown in (b)(c) panels of Fig. 1 and Fig. 2 are the suppression factor or nuclear modification factor, To compare theoretical results with the RHIC and LHC data, we may fix one parameter ofq 0 or λ 0 , and then choose different values for another parameter. For given λ 0 the nuclear modification factor decreases with the increasing ofq 0 , while for givenq 0 the nuclear modification factor increases with the increasing of λ 0 . For the two parametersq 0 and λ 0 we fix one parameter and constrain another by χ 2 /d.o.f fitting to data for the nuclear suppression factor. The χ 2 /d.o.f is defined as follows, where V th stands for the theoretical value, V exp denotes the experimental value, t σ 2 t gives the quadratic sum over all types of errors that one chosen point has, and N the number of data points selected.
In numerical calculations the jet transport parameter q 0 and the mean free path λ 0 are two independent inputs. We choose for a quark jetq 0 = 0.1 -3.0 GeV 2 /fm and λ 0 = 0.1 -1.0 fm, while for a gluon jet the values are correspondingly multiplied by 9/4 forq 0 and 4/9 for λ 0 because of different color factors in gluon-gluon and quarkgluon interacting vertex. From simultaneous χ 2 /d.o.f fits to experimental data at RHIC and LHC shown in Fig. 3, one can extract values of the jet transport parameterq 0 and the mean free path λ 0 at the center of the most central A + A collisions with the given initial time τ 0 = 0.6 fm. For a energetic quark jet, the best fits to the combined PHENIX data [63][64][65] giveq 0 = 1.1±0.30 GeV 2 /fm and λ 0 = 0.4 ± 0.03 fm in 0-5% central Au + Au collisions at √ s N N = 200 GeV, while the best fits to the combined ALICE [6] and CMS [5] data lead toq 0 ≈ 1.7 ± 0.3 GeV 2 /fm, and λ 0 ≈ 0.5 ± 0.05 in 0-5% central Pb+Pb collisions at √ s N N = 2.76 TeV.

IV. DISCUSSIONS
In general, the jet transport parameter should depend on the scale as shown by recent studies on the renormalization of the jet transport parameter [66][67][68]. In our numerical simulations for the initial values forq 0 and λ 0 given by Eq. (6) and Eq. (8), we assume they are constants for different jet transverse momentums as a reasonable approximation for phenomenological studies at the RHIC and the LHC. Note that the best fits shown in Fig. 3 are obtained for hadrons with p T = 5-20 GeV at the RHIC while p T = 10-100 GeV at the LHC, so what we constrain forq 0 and λ 0 may be understood as the averaged values for jets with different transverse momentum. Roughly speaking, what we constrain forq 0 and λ 0 should depend on much greater transverse momentum at the LHC than at the RHIC because of the much wider kinematical region of jet p T at the LHC.
In the formulation for the medium-modified fragmentation functions in Eq. (4), the final-state medium effect of jet quenching is controlled both by the total energy loss ∆E ∝q 0 in Eq. (5) and the multiple scattering number L λ ∝ 1 λ0 in Eq. (8). Therefore the suppression factor R AA is quantified by the two independent parametersq 0 and λ 0 . The trend for the simultaneous χ 2 /d.o.f fits in Fig. 3 shows that an increasingq 0 must associate with an increasing λ 0 to fit well the data at both the RHIC and the LHC. In fact, a larger λ 0 gives a smaller scattering number, and then a largerq 0 is needed to release greater energy loss per scattering in order to describe experimental data. This implicit relation between the two parameters is consistent with theoretical estimates for the jet transport parameter and the mean free path which are related each other via the local temperature in a weakly-coupled QCD medium [25,69].
Of interest are the two different limits as demonstrated in Fig. 3, the single scattering limit with large λ 0 , e.g. λ 0 = 0.7 fm at RHIC, and the infinite number scattering limit with very small λ 0 , e.g λ 0 = 0.1 fm at LHC. The numerical simulations for the simultaneous χ 2 /d.o.f fits at both RHIC and LHC show that in the single scattering limit the suppression factor R AA is insensitive tô q 0 and sensitive to λ 0 , whereas in the infinite number scattering limit R AA is sensitive toq 0 and insensitive to λ 0 . According to an assumption [44,45] for parton scattering obeying a Poisson distribution, the probability for those partons escaping the system without suffering any inelastic scattering is exp(− L λ ), while the probability for partons encountering at least one inelastic scattering gives 1 − exp(− L λ ). One can see these two weight factors in the medium-modified fragmentation function in Eq. (4). In the infinite number scattering limit with small λ 0 , exp(− L λ ) is very small with large L λ , the first term of Eq. (4) with dependence onq 0 will dominate the total fragmentation contribution, so R AA is sensitive tô q 0 and less insensitive to λ 0 . On the other hand, in single scattering limit with large λ 0 , the second term of Eq. (4) gives the dominant contribution, thus R AA is insensitive toq 0 and more sensitive to λ 0 . We observe that our best fits forq 0 and λ 0 are found in the region between the single scattering limit and the infinite number scattering limit due to competing effect between the energy loss per scattering quantified byq 0 and the scattering number quantified by λ 0 , which implies that the data favor a regime of mean-free-paths that suggests multiple scattering in the medium.
From Fig. 3 we can extractq 0 range of values for energetic quarks as constrained by the measured suppression factors of single hadron spectra at RHIC and LHC as follows: at the highest temperatures reached in the most central Au+Au collisions at RHIC and Pb+Pb collisions at LHC. As shown in Fig. 4 for the scaled jet transport parameter q/T 3 , our result falls within the range ofq 0 /T 3 0 for energetic quarks extracted from experimental data on R AA by Jet Collaboration though it is considerably smaller than that given by a strong-coupled AdS/CFT calculation [30,31] as well as a lattice calculation [32,33].
In addition, from Fig. 3 one can extract λ 0 range of values for energetic quarks as constrained by the measured suppression factors of single hadron spectra at RHIC and LHC as: In a theoretical estimate [69] for the mean free path, 1/λ g = ρσ = 3α s (Q 2 )T for which the elastic cross section σ is used at leading order and the density ρ is for an ideal gas. One can introduce K factor to account for higher order correction and the more realistic interaction among the medium particles [70,71], Considering λ q = 9 4 λ g , and assuming the scale Q 2 = ET for a hard parton with energy E traversing a hot QCD medium with temperature T , we find with K = 2.5 -4.0 λ q given by above equation is equal to our best fit for the mean free path at the highest temperatures in both RHIC and LHC. The K factor is bigger than what would be naturally expected, which might be caused by LO σ as well as the ideal gas density ρ in the theoretical evaluation of 1/λ g = ρσ. Higher order correction for the cross section may provide a factor of ∼ 2, while other effects such as corrections due to the difference between the real dynamics of the QGP and the simple picture of an ideal gas may account for the remaining enhancement to K. For instance, a strongly interacting QGP may give a larger cross section than a weakly-coupled QGP. Thus the comparison of the model simulation with the data seems imply that the hot QCD medium at the RHIC and LHC is more likely a strongly interacting medium, which is surely model-dependent and further validations from other observables will be needed for a robust conclusion. It is noted that in numerical estimates we use parton energy E = 8 -25 GeV for p T = 5 -20 GeV hadron production at RHIC while E = 15 -120 GeV for p T = 10-100 GeV hadron production at LHC, and therefore the running coupling α s (Q 2 ) is appreciably smaller at LHC than at RHIC. The phenomenological model given by Eq. (4) assumes that one scattering will induce one gluon emission from the propagating parton, so for a given propagating parton the total scattering number equals to the total number of gluon emissions from this parton. Recent theoretical calculation gives the averaged number of gluon emissions N g from a propagating parton in HT-BW approach within the high-twist framework of parton energy loss [34,72]. In the HT-BW model, the mediummodified FFs are given by numerically solving a set of modified DGLAP evolution equations within the hightwist approach with an initial condition given by Poisson convolution of multiple gluon radiations, which has been shown [72] to give the best agreement with data for the nuclear modification factor R AA in high-energy heavy-ion collisions. Especially, the averaged number of gluon emissions N g from a propagating parton is given [72] in the study for modified DGLAP evolution equations, which can be compared with our extracted number of mediuminduced emissions L λ . Shown in Fig. 5 is the comparison for gluon emission number between our model (solid and dash curves) and the HT-BW approach (dot and dotted-dash curves denoted as "HT-BW"), where the initial quark jets are produced in the point (x, y = 0) of x axis and propagate along +x direction in the transverse plane to escape off the fire ball. The quark transverse momentum is for example chosen as p jet T = 10 GeV for RHIC and 30 GeV for LHC in central A+A collsions. Our results for the averaged number of gluon emissions are consistent with the HT-BW method, and justify the validity of the model as shown in Ref. [17,19].
According to definitions for the jet transport parameter and the mean free path [25], one can estimate the average transverse momentum broadening squared, Then our best fitting values forq 0 and λ 0 give, q 2 T =qλ ≈ 0.44 ± 0.11 0.85 ± 0.20 GeV 2 at T=373 MeV, T=473 MeV, for energetic quarks with one scattering at the initial time τ 0 in the center of the fireball, as shown in Fig. 6. Our numerical results show that for energetic parton jets scattering inside the bulk medium at the highest temperature, the average transverse momentum broadening squared at LHC is about twice of that at RHIC. Compared to initial parton jet energy, the broadening is moderate, which implies that the jet may traverse through the medium with small reflection and justifies the eikonal approximation usually used in jet quenching calculations. As we stated before the AKK FFs in vacuum are used in our numerical simulations. It is noted that a recent theoretical study [73] has confronted seven sets of NLO FF parameterizations with inclusive chargedparticle spectra in p+p collisions at the LHC and identified that most of the theoretical predictions including AKK08 tend to overpredict the measured cross sections by up to a factor of two due to the too-hard gluon-tohadron FFs. In this paper we focus on the medium properties demonstrated by the nuclear modification factor R AA which is a ratio of spectra between A + A and p + p collisions and therefore is expected not to be very sensitive to the choice of FFs parametrization as well as the scale. We have redone our simulations with Kretzer parametrization of FFs [74], which show the extractedq 0 (λ 0 ) is less (larger) about 10-20% by using AKK08 FFs than by using Kretzer FFs.

V. SUMMARY
We have used the NLO pQCD parton model with effective modified fragmentation functions due to radia-tive parton energy loss to study single hadron spectra in high-energy heavy-ion collisions at both RHIC and LHC. The energy loss of the hard partons is incorporated in the modified fragmentation functions which utilize two most important parameters to characterize the properties of the bulk medium, the jet transport parameterq 0 and the mean free path λ 0 both at the initial time τ 0 . We perform the phenomenological study of the experimental data for R AA (p T ) to constrain the two parameters with simultaneous χ 2 /d.o.f fits to RHIC as well as LHC data, and obtain for energetic quarksq 0 ≈ 1.1 ± 0.2 GeV 2 /fm and λ 0 ≈ 0.4 ± 0.03 fm in central Au + Au collisions at √ s N N = 200 GeV, whileq 0 ≈ 1.7 ± 0.3 GeV 2 /fm, and λ 0 ≈ 0.5 ± 0.05 fm in central P b + P b collisions at √ s N N = 2.76 TeV. Numerical analysis shows that the best fit falls between the single scattering limit and multiple scattering limit for the energetic jets propagating through the bulk medium. These results indicate that the average transverse momentum broadening squared q 2 T =qλ of energetic partons for one scattering at initial time τ 0 in the center of the fireball at LHC, q 2 T LHC ≈ 0.85 GeV 2 , which is twice of q 2 T RHIC ≈ 0.44 GeV 2 at RHIC.