Elliptic Flow in Small Systems due to Elliptic Gluon Distributions?

Yoshikazu Hagiwara; Yoshitaka Hatta; Bo-Wen Xiao; Feng Yuan

arXiv:1701.04254·hep-ph·June 14, 2017

Elliptic Flow in Small Systems due to Elliptic Gluon Distributions?

Yoshikazu Hagiwara, Yoshitaka Hatta, Bo-Wen Xiao, Feng Yuan

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TL;DR

This paper explores how elliptic gluon Wigner distributions influence particle correlations in high-energy proton-nucleus collisions, providing a potential explanation for observed elliptic flow phenomena.

Contribution

It introduces a novel application of elliptic gluon Wigner distributions to explain azimuthal correlations in small systems using the double parton scattering mechanism.

Findings

01

Qualitative agreement with experimental $v_2$ data

02

Highlights the role of elliptic gluon distributions in small system flow

03

Encourages further rigorous studies of gluon Wigner functions

Abstract

We investigate the contributions from the so-called elliptic gluon Wigner distributions to the rapidity and azimuthal correlations of particles produced in high energy $p A$ collisions by applying the double parton scattering mechanism. We compute the `elliptic flow' parameter $v_{2}$ as a function of the transverse momentum and rapidity, and find qualitative agreement with experimental observations. This shall encourage further developments with more rigorous studies of the elliptic gluon distributions and their applications in hard scattering processes in $pp$ and $p A$ collisions.

Equations22

\frac{d σ}{d y _{1} d ^{2} k _{1 ⊥} d y _{2} d ^{2} k _{2 ⊥}}_{D P S}

\frac{d σ}{d y _{1} d ^{2} k _{1 ⊥} d y _{2} d ^{2} k _{2 ⊥}}_{D P S}

= \int d^{2} x_{⊥} d^{2} y_{⊥} d^{2} b_{1 ⊥} d^{2} b_{2 ⊥} e^{i k_{1 ⊥} \cdot x_{⊥}} e^{i k_{2 ⊥} \cdot y_{⊥}} F_{A} (x_{p}, x_{p}^{'}; z_{⊥}) F_{B} (x_{A}, x_{A}^{'}; b_{1 ⊥}, b_{2 ⊥}; x_{⊥}, y_{⊥}),

F_{B} \approx S_{x_{A}} (b_{1 ⊥}, x_{⊥}) S_{x_{A}^{'}} (b_{2 ⊥}, y_{⊥}),

F_{B} \approx S_{x_{A}} (b_{1 ⊥}, x_{⊥}) S_{x_{A}^{'}} (b_{2 ⊥}, y_{⊥}),

\frac{d σ}{d y _{1} d ^{2} k _{1 ⊥} d y _{2} d ^{2} k _{2 ⊥}}_{D P S} = \int d^{2} b_{1 ⊥} d^{2} b_{2 ⊥} F_{A} (x_{p}, x_{p}^{'}; z_{⊥}) G_{x_{A}} (b_{1 ⊥}, k_{1 ⊥}) G_{x_{A}^{'}} (b_{2 ⊥}, k_{2 ⊥}),

\frac{d σ}{d y _{1} d ^{2} k _{1 ⊥} d y _{2} d ^{2} k _{2 ⊥}}_{D P S} = \int d^{2} b_{1 ⊥} d^{2} b_{2 ⊥} F_{A} (x_{p}, x_{p}^{'}; z_{⊥}) G_{x_{A}} (b_{1 ⊥}, k_{1 ⊥}) G_{x_{A}^{'}} (b_{2 ⊥}, k_{2 ⊥}),

G (b_{⊥}, k_{⊥}) = G^{0} (b_{⊥}, k_{⊥}) + 2 cos 2 (ϕ_{b} - ϕ_{k}) G (b_{⊥}, k_{⊥}) + \dots .

G (b_{⊥}, k_{⊥}) = G^{0} (b_{⊥}, k_{⊥}) + 2 cos 2 (ϕ_{b} - ϕ_{k}) G (b_{⊥}, k_{⊥}) + \dots .

\int d^{2} z_{⊥} F_{A} (x_{p}, x_{p}^{'}; z_{⊥}) = D_{p} (x_{p}, x_{p}^{'}),

\int d^{2} z_{⊥} F_{A} (x_{p}, x_{p}^{'}; z_{⊥}) = D_{p} (x_{p}, x_{p}^{'}),

\frac{d σ}{d y _{1} d ^{2} k _{1 ⊥} d y _{2} d ^{2} k _{2 ⊥}}_{D P S} \sim \int_{1/Λ} d^{2} b_{⊥} f (x_{p}) f (x_{p}^{'}) G_{x_{A}} (b_{⊥}, k_{1 ⊥}) G_{x_{A}^{'}} (b_{⊥}, k_{2 ⊥})

\frac{d σ}{d y _{1} d ^{2} k _{1 ⊥} d y _{2} d ^{2} k _{2 ⊥}}_{D P S} \sim \int_{1/Λ} d^{2} b_{⊥} f (x_{p}) f (x_{p}^{'}) G_{x_{A}} (b_{⊥}, k_{1 ⊥}) G_{x_{A}^{'}} (b_{⊥}, k_{2 ⊥})

\propto π \int_{1/Λ} d b_{⊥}^{2} [G_{x_{A}}^{0} (b_{⊥}, k_{1 ⊥}) G_{x_{A}^{'}}^{0} (b_{⊥}, k_{2 ⊥}) + 2 cos 2 (ϕ_{k_{1 ⊥}} - ϕ_{k_{2 ⊥}}) G_{x_{A}} (b_{⊥}, k_{1 ⊥}) G_{x_{A}^{'}} (b_{⊥}, k_{2 ⊥})] .

\int^{1/Λ} d^{2} b_{1 ⊥} d^{2} b_{2 ⊥} e^{- Λ^{2} ∣ b_{1 ⊥} - b_{2 ⊥} ∣^{2}} G_{x_{A}} (b_{1 ⊥}, k_{1 ⊥}) G_{x_{A}^{'}} (b_{2 ⊥}, k_{2 ⊥})

\int^{1/Λ} d^{2} b_{1 ⊥} d^{2} b_{2 ⊥} e^{- Λ^{2} ∣ b_{1 ⊥} - b_{2 ⊥} ∣^{2}} G_{x_{A}} (b_{1 ⊥}, k_{1 ⊥}) G_{x_{A}^{'}} (b_{2 ⊥}, k_{2 ⊥})

\displaystyle=4\pi^{2}\int_{0}^{1/\Lambda}b_{1\perp}db_{1\perp}b_{2\perp}db_{2\perp}e^{-\Lambda^{2}(b_{1\perp}^{2}+b_{2\perp}^{2})}\Bigl{[}I_{0}(2\Lambda^{2}b_{1\perp}b_{2\perp})G^{0}_{x_{A}}(b_{1\perp},k_{1\perp})G^{0}_{x_{A}^{\prime}}(b_{2\perp},k_{2\perp})

\displaystyle\qquad\qquad+2\cos 2(\phi_{k_{1\perp}}-\phi_{k_{2\perp}})I_{2}(2\Lambda^{2}b_{1\perp}b_{2\perp})\widetilde{G}_{x_{A}}(b_{1\perp},k_{1\perp})\widetilde{G}_{x_{A}^{\prime}}(b_{2\perp,}k_{2\perp})\Bigr{]}\,.

V_{2} (k_{1 ⊥}, k_{2 ⊥}) \equiv \frac{\int _{0}^{R_{c u t}} b _{1 ⊥} d b _{1 ⊥} b _{2 ⊥} d b _{2 ⊥} e ^{- Λ^{2} (b_{1 ⊥}^{2} + b_{2 ⊥}^{2})} I _{2} ( 2 Λ ^{2} b _{1 ⊥} b _{2 ⊥} ) G _{x_{A}} ( b _{1 ⊥} , k _{1 ⊥} ) G _{x_{A}^{'}} ( b _{2 ⊥} , k _{2 ⊥} )}{\int _{0}^{R_{c u t}} b _{1 ⊥} d b _{1 ⊥} b _{2 ⊥} d b _{2 ⊥} e ^{- Λ^{2} (b_{1 ⊥}^{2} + b_{2 ⊥}^{2})} I _{0} ( 2 Λ ^{2} b _{1 ⊥} b _{2 ⊥} ) G _{x_{A}}^{0} ( b _{1 ⊥} , k _{1 ⊥} ) G _{x_{A}^{'}}^{0} ( b _{2 ⊥} , k _{2 ⊥} )},

V_{2} (k_{1 ⊥}, k_{2 ⊥}) \equiv \frac{\int _{0}^{R_{c u t}} b _{1 ⊥} d b _{1 ⊥} b _{2 ⊥} d b _{2 ⊥} e ^{- Λ^{2} (b_{1 ⊥}^{2} + b_{2 ⊥}^{2})} I _{2} ( 2 Λ ^{2} b _{1 ⊥} b _{2 ⊥} ) G _{x_{A}} ( b _{1 ⊥} , k _{1 ⊥} ) G _{x_{A}^{'}} ( b _{2 ⊥} , k _{2 ⊥} )}{\int _{0}^{R_{c u t}} b _{1 ⊥} d b _{1 ⊥} b _{2 ⊥} d b _{2 ⊥} e ^{- Λ^{2} (b_{1 ⊥}^{2} + b_{2 ⊥}^{2})} I _{0} ( 2 Λ ^{2} b _{1 ⊥} b _{2 ⊥} ) G _{x_{A}}^{0} ( b _{1 ⊥} , k _{1 ⊥} ) G _{x_{A}^{'}}^{0} ( b _{2 ⊥} , k _{2 ⊥} )},

v_{2} (k_{⊥}, k_{⊥}^{r e f}) \equiv \frac{V _{2} ( k _{⊥} , k _{⊥}^{r e f} )}{V _{2} ( k _{⊥}^{r e f} , k _{⊥}^{r e f} )},

v_{2} (k_{⊥}, k_{⊥}^{r e f}) \equiv \frac{V _{2} ( k _{⊥} , k _{⊥}^{r e f} )}{V _{2} ( k _{⊥}^{r e f} , k _{⊥}^{r e f} )},

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Full text

Elliptic Flow in Small Systems due to Elliptic Gluon Distributions?

Yoshikazu Hagiwara

Department of Physics, Kyoto University, Kyoto 606-8502, Japan

Yoshitaka Hatta

Yukawa Institute for Theoretical Physics, Kyoto University, Kyoto 606-8502, Japan

Bo-Wen Xiao

Key Laboratory of Quark and Lepton Physics (MOE) and Institute of Particle Physics, Central China Normal University, Wuhan 430079, China

Feng Yuan

Nuclear Science Division, Lawrence Berkeley National Laboratory, Berkeley, CA 94720, USA

Abstract

We investigate the contributions from the so-called elliptic gluon Wigner distributions to the rapidity and azimuthal correlations of particles produced in high energy $pp$ and $pA$ collisions by applying the double parton scattering mechanism. We compute the ‘elliptic flow’ parameter $v_{2}$ as a function of the transverse momentum and rapidity, and find qualitative agreement with experimental observations. This shall encourage further developments with more rigorous studies of the elliptic gluon distributions and their applications in hard scattering processes in $pp$ and $pA$ collisions.

pacs:

24.85.+p, 12.38.Bx, 12.39.St

††preprint: YITP-17-02

I Introduction

One of the interesting experimental observations from the proton-proton and proton-nucleus collisions at the Large Hadron Collider (LHC) and Relativistic Heavy Ion Collider (RHIC) is the long range rapidity and azimuthal angle correlations between hadrons Khachatryan:2010gv ; Abelev:2012ola ; Aad:2012gla ; CMS:2012qk ; Adare:2014keg ; Adare:2015ctn ; Aad:2014lta ; Aad:2015gqa ; Aaboud:2016yar , see, e.g., a recent review in Ref. Dusling:2015gta . These intriguing observations have generated great theoretical investigations, and many models have been proposed to explain the experimental results, including (but not limited to) hydrodynamics dEnterria:2010xip ; CasalderreySolana:2009uk ; Avsar:2010rf ; Schenke:2014zha ; Yan:2013laa , QCD motivated models Kopeliovich:2007fv ; Kopeliovich:2008nx ; Gyulassy:2014cfa ; Gambini:2016ijt , and in particular, the multi-gluon correlations calculated in the Color Glass Condensate (CGC) framework Kovner:2010xk ; Kovner:2011pe ; Dusling:2012wy ; Dusling:2012cg ; Kovchegov:2012nd ; Iancu:2013uva ; Schenke:2015aqa ; Dumitru:2014dra ; Dumitru:2010mv ; Dumitru:2014yza ; Lappi:2015vha ; Levin:2011fb ; Gotsman:2016whc ; Lappi:2015vta .

In this paper, we investigate the contribution from the double parton scattering (DPS) Diehl:2011yj ; Manohar:2012pe coupled with the so-called elliptic gluon Wigner distribution Hatta:2016dxp ; Hagiwara:2016kam ; Zhou:2016rnt . In high energy collisions, we expect the DPS, or in general, the multi-parton scattering, is the dominant source for multi-particle productions. A unique feature of DPS is that its contribution is not strongly suppressed for near-side particle productions with large rapidity separation as compared to the single parton scattering (SPS) contribution. Therefore, DPS may well be the dominant source for long range correlations among produced hadrons.

It was first pointed out in Ref. Strikman:2010bg that the DPS plays an important role in two particle production in forward $pA$ and $dA$ collisions at RHIC. This idea was followed up in the saturation formalism in Ref. Stasto:2011ru to estimate the so-called pedestal contribution in the correlation measurements. Further study in Ref. Lappi:2012nh also confirmed the importance of these contributions in the two particle production in $pA$ collisions. However, all these studies assumed that the two hard scatterings are essentially uncorrelated. In the following, we will extend the DPS mechanism to include the impact parameter dependence which naturally encodes the correlation between the two scatterings. If we average over the impact parameter space, this will reduce to the previous applications of the DPS mechanism in the CGC framework. However, the unintegrated gluon distribution involved in these scatterings depends on the impact parameter. In particular, there is a nonzero $\cos(2\phi)$ azimuthal correlation between the transverse momentum $k_{\perp}$ and the impact parameter $b_{\perp}$ , which was referred to as the elliptic gluon Wigner distribution in Ref. Hatta:2016dxp . Since the impact parameters for the two hard scatterings are correlated due to the DPS mechanism, we expect the transverse momenta from the two hard scatterings are correlated as well. This will naturally give rise to the $\cos(2\phi)$ two-particle correlation in the final state.

In Ref. Hatta:2016dxp , the elliptic gluon Wigner distribution has been shown to be measurable in diffractive dijet production in lepton-nucleon collisions at the future electron-ion collider (EIC). The present study suggests that the same distribution can affect various observables in different types of collisions.

The rest of this paper is organized as follows. In Sec. II, we study the DPS contributions to the two particle production in the dilute-dense collisions and derive a formula for the ‘elliptic flow’ parameter $v_{2}$ . The result is relevant to $pp$ and $pA$ experiments at RHIC and the LHC. In Sec. III, we numerically evaluate $v_{2}$ in a model which incorporates the saturation effect in the target. We point out some generic features of the DPS contributions which can be compared to the experimental observations. We summarize our paper in Sec. IV.

II Double Parton Scattering Contributions in the Dilute-Dense Collisions

In order to describe the near-side two particle correlations in $pp$ and $pA$ collisions, we introduce the impact parameter dependence in the DPS framework. Similarly to the derivation of DPS in Refs. Diehl:2011yj ; Manohar:2012pe , we write down the generic expression for the differential cross section of two parton production as

[TABLE]

where $z_{\perp}=|\vec{b}_{1\perp}-\vec{b}_{2\perp}|$ , and $\vec{b}_{1\perp}$ and $\vec{b}_{2\perp}$ denote the two hard scattering positions with respect to the center of the target. The ‘dipole sizes’ $x_{\perp}$ and $y_{\perp}$ are Fourier-conjugate variables to the partons’ outgoing transverse momentum $k_{1\perp}$ and $k_{2\perp}$ , respectively. The longitudinal momentum fractions $x_{p}$ , $x_{p}^{\prime}$ , $x_{A}$ , and $x_{A}^{\prime}$ are determined by the final state kinematics. The physics picture is that two partons from the incoming proton encounter multiple scattering off the target, and fragment into two final state particles. The multiple scattering is described in the CGC framework or in the color-dipole model. For a large nucleus, we can assume a factorized form

[TABLE]

where $S$ is the dipole S-matrix which may be in the fundamental or adjoint representation depending on the partonic channels involved in the DPS. The terms neglected in (2) are of order $1/N_{c}^{2}$ . It has been argued Lappi:2015vta that these color-suppressed, but ‘connected’ contributions can give rise to nonvanishing $v_{2}$ in $pp$ and $pA$ collisions. Moreover, if the the target is small, as in $pp$ collisions, factorization (2) is violated even in the large- $N_{c}$ limit due to the small- $x$ evolution in the target. (In the case of a dipole target, this can be shown analytically Hatta:2007fg ; Avsar:2008ph .) Such factorization breaking effects have been considered as another source of $v_{2}$ in small systems Kovner:2010xk ; Kovner:2011pe ; Kovner:2012jm .

Here we show that, even if the factorization (2) holds strictly, there exist non-trivial angular correlations between the two outgoing particles due to the angular correlation between $\vec{b}_{1_{\perp}}$ and $\vec{x}_{\perp}$ in the $S$ -matrix. It should be mentioned that the idea that the correlation between impact parameter and dipole orientation generates anisotropy in the final state has been previously studied in the context of single Kopeliovich:2007fv ; Kopeliovich:2008nx (see also, Iancu:2017fzn ) and double Levin:2011fb ; Gotsman:2016whc parton scattering. Thus, the approach here is essentially the same as in Levin:2011fb ; Gotsman:2016whc . Yet, our formulation is considerably more concise and clearly establishes the connection to the elliptic gluon Wigner distribution which is a fundamental object in the tomographic study of the nucleon/nucleus.

For this purpose, let us write (1) as

[TABLE]

where $G(\vec{b}_{\perp},\vec{k}_{\perp})$ is the Fourier transform of $S(\vec{b}_{\perp},\vec{x}_{\perp})$ and we assumed (2). The angular correlation between $\vec{b}_{\perp}$ and $\vec{x}_{\perp}$ is transformed into the one between $\vec{b}_{\perp}$ and $\vec{k}_{\perp}$ . At small- $x$ , this correlation is dominantly elliptic Hatta:2016dxp ; Hagiwara:2016kam , namely,

[TABLE]

The angular integrals in (3) then lead to an elliptic angular correlation of the form $\cos 2(\phi_{k_{1}}-\phi_{k_{2}})$ .

This can be seen most clearly and model-independently at large impact parameter where it is convenient to write $\vec{b}_{1,2\perp}=\vec{b}_{\perp}\pm\vec{z}_{\perp}/2$ , so that $d^{2}b_{1\perp}d^{2}b_{2\perp}=d^{2}z_{\perp}d^{2}b_{\perp}$ . Since the two partons are confined in the proton, the $z_{\perp}$ integral is limited within the confinement radius $z_{\perp}\lesssim 1/\Lambda$ . When $b_{\perp}\gg 1/\Lambda\sim z_{\perp}$ , we can approximately integrate over $z_{\perp}$ to obtain the collinear double parton distribution of the proton,

[TABLE]

which can be further simplified as ${\cal D}_{p}(x_{p},x_{p}^{\prime})={\cal C}(x_{p},x_{p}^{\prime})f(x_{p})f(x_{p}^{\prime})$ with ${\cal C}\approx 1$ . With this approximation, we can write down the differential cross section as

[TABLE]

As expected, we recognize the $\cos 2(\phi_{k_{1}}-\phi_{k_{2}})$ correlation proportional to the elliptic part $\widetilde{G}$ squared.

We now turn to the small impact parameter region $b_{\perp}\sim z_{\perp}\sim 1/\Lambda$ . To proceed, we introduce a Gaussian model $F_{A}(z_{\perp})\propto e^{-z_{\perp}^{2}\Lambda^{2}}$ . The angular integrals can then be performed as

[TABLE]

We again find the elliptic correlation $\cos 2(\phi_{k_{1}}-\phi_{k_{2}})$ . Other models of $F_{A}$ will also give rise to this correlation, as long as $F_{A}$ depends on the angle between $\vec{b}_{1\perp}$ and $\vec{b}_{2\perp}$ via $z_{\perp}=|\vec{b}_{1\perp}-\vec{b}_{2\perp}|$ .

Noting that the upper limit of the $b_{1,2\perp}$ -integrations in (7) can actually be extended to some value $R_{cut}>1/\Lambda$ , we define

[TABLE]

This is related to the experimentally measured $v_{2}$ via

[TABLE]

where $k_{\perp}^{ref}$ denotes some reference momentum. Experimentally, it has been observed that $v_{2}$ is roughly independent of $k_{\perp}^{ref}$ . This implies that the two-particle correlation $V_{2}$ factorizes $V_{2}(k_{1\perp},k_{2\perp})\approx v_{2}(k_{1\perp})v_{2}(k_{2\perp})$ , and this is consistent with the hydrodynamic interpretation of $v_{2}$ . In our case (8), the integrand approximately factorizes at small $b_{1,2\perp}$ . However, the result after the full $b_{1,2\perp}$ -integrations does not factorize in general.

III Model calculation

To illustrate the DPS contribution discussed above, we evaluate (8) in a model that incorporates the gluon saturation effect at small- $x$ . For definiteness, we consider the $pp$ collisions partly because realistic models for $pA$ with both the $b_{\perp}$ -dependence and the small- $x$ evolution are not available to us. The angular independent part $G^{0}$ and the elliptic part $\widetilde{G}$ are computed from the solution of the impact parameter dependent Balitsky-Kovchegov (BK) equation in the same way as explained in Hagiwara:2016kam . The only difference is that here we use a different initial condition to be slightly more realistic ( $e^{-d^{2}}\to e^{-cd^{2}}$ with $c=6$ in Eq. (7) of Hagiwara:2016kam ). For small dipole sizes $r_{\perp}\to 0$ and at small impact parameter $b_{\perp}\approx 0$ , this gives the initial condition $S_{Y=0}(b_{\perp},r_{\perp})\approx e^{-cr_{\perp}^{2}/R^{2}}$ where $R$ is roughly the size of the target. For the proton, we use $R=1\,$ fm so that the initial condition is $\sim e^{-r_{\perp}^{2}/(0.4{\rm fm})^{2}}$ which is the same as the original GBW model GolecBiernat:1998js . Below we use $R$ as the unit of length, so for example $R_{cut}=2$ means $R_{cut}=2R$ . The current numerical result is intended to be viewed as an illustrative example which shows that this mechanism due to the elliptic Wigner distribution can generate sizeable elliptic flow in small systems. Of course, a more realistic numerical model calculation should be carried out in the future in order to compare with the experimental data measured for small systems created in $pp$ and $pA$ collisions.

The results for $k_{\perp}=k_{\perp}^{ref}$ and $x_{A}=x_{A^{\prime}}=e^{-Y}$ are shown in Fig. 1 for different values of $Y$ with $\Lambda=1$ . In the two figures, we used different values of the cutoff $R_{cut}$ in the $b_{\perp}$ -integral. Actually, the elliptic part $\widetilde{G}$ becomes negative in the large- $k_{\perp}$ region. This means that the squared function $(\tilde{G})^{2}$ in the numerator has two peaks in the $k_{\perp}$ direction at fixed $b_{1\perp}\approx b_{2\perp}$ . However, the zero of $\tilde{G}$ is $b_{\perp}$ -dependent, so that after integrating over $b_{\perp}$ we obtain the single-peak structure as in the right figure. On the other hand, if the cutoff is small as in the left figure, $b_{\perp}$ -averaging is insufficient and we see a remnant of the double-peak structure. Note that the peak position of $v_{2}$ is almost independent of $Y$ , and does not coincide with the saturation momentum $k\sim Q_{s}(Y)$ which is a rapidly increasing function of $Y$ . This is a characteristic property of the elliptic part $\widetilde{G}$ observed in Hagiwara:2016kam . Interestingly, Ref. Kovner:2012jm argued that the peak position of $v_{2}$ from the present mechanism should occur at the inverse correlation length of $Q_{s}$ in the transverse plane which is much smaller than $Q_{s}$ . It remains to be seen whether the observation in Hagiwara:2016kam can be physically interpreted as such. We also note that the height of the peak decreases with increasing $Y$ largely because $\widetilde{G}$ has the same property. Compared with the experimental data, the magnitude of $v_{2}$ in our model is somewhat smaller even for the smallest values of $Y$ .

Next we test the degree of factorization. We choose $k_{\perp}\neq k_{\perp}^{ref}$ and check the $k_{\perp}^{ref}$ -dependence of the result. The integrand of (8) factorizes at small $b_{\perp}$ , because $I_{2}(2\Lambda^{2}b_{1\perp}b_{2\perp})\sim(b_{1\perp}b_{2\perp})^{2}$ . Thus, factorization is good if $R_{cut}$ is small and this is clearly seen in Fig. 2 ( $Y=4$ ) and Fig 3 ( $Y=8$ ). We also see that the factorization holds better for larger $Y$ values. Note that $v_{2}$ is no longer positive definite once we allow $k_{\perp}\neq k_{\perp}^{ref}$ because $\widetilde{G}$ is negative for large $k_{\perp}^{ref}$ . When $Y$ becomes large, the negative region of $\widetilde{G}$ is pushed to a larger $k$ -region and $v_{2}$ tends to become positive.

Finally we study the rapidity correlation between two particles. We take $x_{A}$ and $x_{A^{\prime}}$ in (8) to be different and compute $v_{2}(k_{\perp}=k_{\perp}^{ref}=2)$ from (9) as a function of $\Delta Y=Y-Y^{ref}=\ln\frac{1}{x}-\ln\frac{1}{x^{ref}}$ . (In practice we set $Y^{ref}=0$ .) The result is shown in Fig. 4. We recognize a certain degree of ‘long-range rapidity correlation’, namely, $v_{2}$ decreases only slowly with increasing $\Delta Y$ . This is largely due to approximate factorization of the double scattering amplitude (2). We should mention that when $\Delta Y$ becomes too large such that $\alpha_{s}\Delta Y\sim 1$ , one has to consider the small- $x$ evolution between the two rapidities Iancu:2013uva . This is however beyond the scope of this work.

IV Conclusions and Discussions

To summarize, we have explored the two-particle productions in small systems created in high energy $pp$ and $pA$ collisions from the double parton scattering mechanism, where the elliptic gluon Wigner distributions give rise to the desired $\cos(2\phi)$ azimuthal angular correlations. By applying the DPS idea, we derived a formula for the two particle correlation in the small- $x$ saturation formalism, where two partons from the incoming nucleon scatter with the target nucleon/nucleus and produce two particles in the final state. The DPS mechanism imposes the impact parameter correlation between the two hard partonic scattering processes, which results in a correlation between the transverse momenta of the final state particles. Due to the unique feature of the DPS mechanism, this correlation will not decrease dramatically with the increase of the rapidity difference between the two particles.

We have also applied a recent result of the elliptic gluon distributions from the BK equation Hagiwara:2016kam to illustrate their contributions to the $\cos(2\phi)$ correlation between two particles produced in high energy $pp$ and $pA$ collisions. The size of the elliptic flow parameter $v_{2}$ was found in a similar range as the experimental observations at RHIC and the LHC. This is an encouraging message, and demonstrates that the long range correlation of $v_{2}$ may have significant contributions from the elliptic gluon distributions in the target. However, we would like to emphasize that we have limited knowledge on the elliptic gluon distribution as compared to the usual dipole gluon distribution, and more studies are needed to compare to the experimental data. This will also help to pin down the underlying mechanism for the novel “flow” phenomena in high energy $pp$ and $pA$ collisions.

Finally, we would like to point out that the elliptic gluon Wigner distribution represents a nontrivial tomography structure of gluons inside the nucleon/nucleus. Its dependence on $x$ , $b_{\perp}$ and $k_{\perp}$ will provide not only the imaging of parton distributions at small- $x$ , but also the unique opportunity to explore the QCD dynamics associated with the small- $x$ evolution Hagiwara:2016kam . Since the elliptic gluon distribution can be well studied in hard diffractive dijet production at the EIC Hatta:2016dxp , the comparison between the two particle elliptic flow in $pp$ and $pA$ collisions and further observables in $eA$ collisions will be crucial to understand the gluon dynamics under extreme conditions. We hope to come back to this issue soon.

Acknowledgements.

We thank Edmond Iancu and Amir Rezaeian for correspondence about their related work Iancu:2017fzn . This material is based upon work supported by the U.S. Department of Energy, Office of Science, Office of Nuclear Physics, under contract number DE-AC02-05CH11231 and by the Natural Science Foundation of China (NSFC) under Grant No. 11575070.

Bibliography46

The reference list from the paper itself. Each links out to its DOI / PubMed record.

1(1) V. Khachatryan et al. [CMS Collaboration], JHEP 1009 , 091 (2010) doi:10.1007/JHEP 09(2010)091 [ar Xiv:1009.4122 [hep-ex]].
2(2) B. Abelev et al. [ALICE Collaboration], Phys. Lett. B 719 , 29 (2013) doi:10.1016/j.physletb.2013.01.012 [ar Xiv:1212.2001 [nucl-ex]].
3(3) G. Aad et al. [ATLAS Collaboration], Phys. Rev. Lett. 110 , no. 18, 182302 (2013) doi:10.1103/Phys Rev Lett.110.182302 [ar Xiv:1212.5198 [hep-ex]].
4(4) S. Chatrchyan et al. [CMS Collaboration], Phys. Lett. B 718 , 795 (2013) doi:10.1016/j.physletb.2012.11.025 [ar Xiv:1210.5482 [nucl-ex]].
5(5) A. Adare et al. [PHENIX Collaboration], Phys. Rev. Lett. 114 , no. 19, 192301 (2015) doi:10.1103/Phys Rev Lett.114.192301 [ar Xiv:1404.7461 [nucl-ex]].
6(6) A. Adare et al. [PHENIX Collaboration], Phys. Rev. Lett. 115 , no. 14, 142301 (2015) doi:10.1103/Phys Rev Lett.115.142301 [ar Xiv:1507.06273 [nucl-ex]].
7(7) G. Aad et al. [ATLAS Collaboration], Phys. Rev. C 90 , no. 4, 044906 (2014) doi:10.1103/Phys Rev C.90.044906 [ar Xiv:1409.1792 [hep-ex]].
8(8) G. Aad et al. [ATLAS Collaboration], Phys. Rev. Lett. 116 , no. 17, 172301 (2016) doi:10.1103/Phys Rev Lett.116.172301 [ar Xiv:1509.04776 [hep-ex]].