Diffractive dijet photoproduction in ultraperipheral collisions at the LHC in next-to-leading order QCD

We make predictions for the cross sections of diffractive dijet photoproduction in pp, pA and AA ultraperipheral collisions (UPCs) at the LHC during Runs 1 and 2 using next-to-leading perturbative QCD. We find that the resulting cross sections are sufficiently large and, compared to lepton-proton scattering at HERA, have an enhanced sensitivity to small observed momentum fractions in the diffractive exchange, commonly denoted zℙjets\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ {z}_{\mathrm{\mathbb{P}}}^{\mathrm{jets}} $$\end{document}, and an unprecedented reach in the invariant mass of the photon-nucleon system W. We examine two competing schemes of diffractive QCD factorization breaking, which assume either a global suppression factor or a suppression for resolved photons only and demonstrate that the two scenarios can be distinguished by the nuclear dependence of the distributions in the observed parton momentum fraction in the photon xγjets.


Introduction
Ultraperipheral collisions (UPCs) of relativistic ions are characterized by large transverse distances (impact parameters) between the centers of the colliding ions, exceeding the sum of their radii. For such collisions, the strong interaction is suppressed and the ions interact electromagnetically through the emission of quasi-real photons [1][2][3][4]. The flux of these photons scales as Z 2 , where Z is the nuclear charge, and has a broad energy spectrum with the maximal photon energy in the laboratory frame scaling as γ L , where γ L is the nuclear Lorentz factor. This allows one to study photon-photon and photon-nucleus scattering at unprecedentedly high energies [5].
The UPC program at the LHC during Run 1 focused primarily on exclusive photoproduction of charmonia, in particular J/ψ and ψ(2S) mesons, which probes the gluon distribution of the target g(x, µ 2 ) at small values of the momentum fraction x and a resolution scale µ 2 = O(few GeV 2 ) [6]. This process was measured in proton-proton (pp) 2 Diffractive dijet photoproduction in proton-proton UPCs at the LHC Feynman graphs for the direct (graph a) and the resolved (graph b) photon contributions to the production of two quark jets.
Considering proton-proton UPCs, A = B = p, the cross section of diffractive dijet photoproduction can be written as a sum of two terms: dσ(pp → p + 2jets + X + Y ) = dσ(pp → p + 2jets + X + Y ) (+) +dσ(pp → p + 2jets + X + Y ) (−) , (2.1) where X stands for the produced diffractive final state X after removing two jets and Y denotes the final state of the diffracting proton, which, besides the elastic state Y = p, may contain hadronic states with low invariant mass. Note that the possibility of the proton diffraction dissociation is not explicitly shown in figure 1. The first and the second terms in eq. (2.1) correspond to the diffracting proton moving along the positive and the negative z-axis, respectively. This reflects the ambiguity common for symmetric UPCs that either of the colliding ions can serve as a photon source and as a target [5]. Since the jet pseudorapidities η 1 and η 2 are usually defined with respect to the direction of the diffracting proton [38], the two terms in eq. (2.1) can be related to each other by inverting the sign of η 1 and η 2 : The cross section dσ(pp → p + 2jets + X + Y ) (+) can be readily written by analogy with the standard expression for the dijet diffractive photoproduction cross section dσ(ep → JHEP04(2016)158 e + 2jets + X + Y ) for lepton-proton scattering, see e.g. [38,39]: where a and b are parton flavors; f γ/p (y) is the flux of equivalent photons of the proton, which depends on the photon light-cone momentum fraction y; f a/γ (x γ , µ 2 ) is the parton distribution function (PDF) of the photon, which depends on the parton light-cone momentum fraction x γ and the factorization scale µ; f D(4) b/p (x P , z P , t, µ 2 ) is the diffractive PDF of the proton; dσ (n) ab→jets is the elementary cross section for the production of an n-parton final state in the interaction of partons a and b; and the sum over a involves quarks and gluons (the resolved photon contribution) and the direct photon contribution with a = γ, which has support at LO only at x γ = 1.
In eq. (2.3), besides the standard expression for ep scattering, we also explicitly introduced the rapidity gap survival factor of S 2 (y) ≤ 1, which takes into account the probability of soft inelastic interactions between the colliding protons, which populate, and thus suppress, the final-state rapidity gaps. The factor of S 2 (y) depends on y and the total invariant energy √ s N N ; in pp UPCs, it can be viewed as a phenomenological factor modifying the photon flux f γ/p (y) [13,40]. The QCD collinear factorization theorem for hard inclusive diffraction [41] allows one to introduce universal diffractive PDFs f D(4) b/p (x P , z P , t, µ 2 ) and to determine them by fitting to the measured diffractive structure functions [42][43][44]. The analysis also shows that for small values of x P , f D(4) b/p (x P , z P , t, µ 2 ) can be written as the product of two factors [45]: f D(4) b/p (x P , z P , t, µ 2 ) = f b/P (z P , µ 2 )f P/p (x P , t) , (2.4) where f b/P (z P , µ 2 ) is the PDF of the Pomeron (the lower blob in figure 1) and f P/p (x P , t) is the Pomeron flux (the double line in figure 1). Note that the word "Pomeron" here denotes the diffractive exchange. Equation (2.4) helps to understand the meaning of the diffractive variables z P , x P and t entering eq. (2.3): z P is the light-cone momentum fraction of a parton in the Pomeron; x P is the light-cone momentum fraction of the Pomeron in the proton; t is the invariant momentum transfer squared.
In the measurements of diffractive dijet photoproduction in ep scattering, the variables y, x P and t are directly reconstructed by detecting the scattered electron, the final proton and the diffractive final state, see e.g. [28]: where p, p Y , k, and q are the four-momenta of the initial proton, the final proton (with the possibility of diffraction dissociation into the state Y ), the initial lepton and the photon,

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respectively; E e , E e , and E X are the energies of the initial lepton, the final lepton, and the diffractive final state X, respectively; P X,z and M X are the z-component of the momentum and the invariant mass of the state X, respectively; and s = (k + p) 2 is the square of the total center-of-mass energy of the collision. In ep scattering at HERA, the limits on y, x P and t are determined by the experimental conditions and cuts. In contrast, in pp UPCs the scattered protons travel along the beam pipe, and, hence, are undetected. As a result, the limits on y, t and x P in eq. (2.3) are determined from general requirements to produce a diffractive final state. The two remaining variables z P and x γ in eq. (2.3) cannot be directly reconstructed by measuring the final state; their values can be compared to the hadron-level estimators z jets P and x jets γ , respectively, which are reconstructed from the measurement of the dijet and the diffractive final state [28]: where the sum jets runs over the hadronic final states labeled "i", which are included in the jets.

Flux of equivalent photons in pp UPCs
The flux of quasi-real photons emitted by a relativistic proton (ion) can be found using the well-known Weizsäcker-Williams (WW) approximation [1-4, 46, 47]. Since one also needs to take into account the charge and magnetization distribution in the proton, in practical applications one often uses approximate expressions [48,49] reproducing the exact result with a few percent accuracy, see the discussion in ref. [50]. The photon flux produced by a relativistic charge Z at the transverse distance b from its center reads, see e.g. [47]: where x is the fraction of the ion energy carried by the photon; α e.m. is the fine-structure constant; F ch (k 2 ⊥ ) is the charge form factor; k ⊥ is the photon transverse momentum; J 1 is the Bessel function of the first kind; and m p is the proton mass. Different expressions for the photon flux used in the literature correspond to various assumptions for F ch (k 2 ⊥ ) and treatments of subleading terms in eq. (2.7).
The integration of f γ/Z (x, b) over all impact parameters gives the following general expression for the photon flux produced by a relativistic ion: (2.8) In our calculations of pp UPCs we will use the result of Drees and Zeppenfeld (DZ) [48]:  Figure 2. Left: the proton and electron photon spectra xf γ/p (x) and xf γ/e (x), respectively, as a function of the energy fraction x. Right: the photon spectra kf γ/p (k) and kf γ/e (k) as a function of the photon energy k in the target rest frame.
where A = 1 + (0.71 GeV 2 )/Q 2 min and Q 2 min = (xm p ) 2 /(1 − x) is the minimal kinematicallyallowed photon virtuality. Alternatively, in the literature one also considers the photon flux produced by a relativistic point-like (PL) charge Z passing a target at a minimum impact parameter b min : where ζ = xm p b min and b min = 0.7 fm for the proton [50]. It is illustrative to compare the photon flux of the proton with that of a relativistic electron [4]: where m e is the electron mass; Q 2 max is the maximal photon virtuality, which is usually determined by the experimental conditions. Figure 2 presents a comparison of the spectrum of equivalent photons of the proton with that of the electron. In the left panel, we show xf γ/p (x) for the proton as a function of x (the red solid and the blue dot-dashed curves corresponding to eqs. (2.9) and (2.10), respectively) and xf γ/e (x) for the electron (the dotted black curve corresponding to eq. (2.11)). One can see from this panel that the energy spectrum for the point-like electron is much flatter than that for the composite proton. The photon energy k scales as γ L m p in the laboratory frame and as 2γ 2 L m p in the target rest frame, where γ L is the Lorentz factor of the emitting ion. The right panel of figure 2 shows the photon spectra kf γ/p (k) and kf γ/e (k) as a function of the photon energy k in the proton target rest frame. For the proton beam, the curves correspond to proton-proton collisions at √ s N N = 7 TeV. For the electron beam, the curve corresponds to the HERA kinematics with the 27.5 GeV electron beam and the 920 GeV proton beam. One can see from the panel that pp UPCs, in principle, allow one to obtain photon energies exceeding those at HERA by two orders of magnitude.

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We explained in section 2.1 that the photon flux f γ/p (x) is somewhat reduced by the rapidity gap survival probability factor of S 2 (x). To estimate it, we use the method of refs. [13,51], where S 2 (x) is calculated as a result of eikonalization of multiple Pomeron exchanges between the colliding protons: where b is the impact parameter; M(x, b) is the diffractive amplitude of the process of interest in the impact parameter space; P (s, b) is the probability to not have the strong inelastic proton-proton interaction at the impact parameter b; and s = s N N for brevity. The probability P (s, b) in the two-channel eikonal model of ref. [51] is where γ = 0.4 and Ω(s, b) is the proton optical density. Assuming that Ω(s, b) has the form of the effective Pomeron exchange trajectory, one obtains: where σ tot pp (s) is the total proton-proton cross section; B P = B 0 /2 + α ln(s/s 0 ) is the slope of the t dependence of the elastic pp amplitude; and the parameter α ≥ 1 results from eikonalized multiple Pomeron exchanges and is found from the requirement: For σ tot pp (s), we use the fit of the Review of Particle Physics [52]. The resulting values of S 2 (x) weakly depend on the exact value of the slope B P ; in our calculation, we used B 0 = 10 GeV −2 and α = 0.25 GeV −2 , which correctly reproduce the slope of the elastic pp cross section at small |t| [51].
For |M(x, b)| 2 in eq. (2.12), we use the photon flux of the proton in the impact parameter space, eq. (2.7), with F ch (Q 2 ) = F p (Q 2 ) = 1/(1 + Q 2 /(0.71 GeV 2 )) 2 . Since the contribution of small impact parameters b < b min ≈ 0.7 fm to the photon flux, eq. (2.7), is small, the integrand in eq. (2.12) receives the dominant contribution from b > b min , where Ω(s, b) is not large. As a result, one expects that the suppression due to S 2 (x) should not be large.
The resulting values of S 2 (x) as a function of the photon light-cone momentum fraction x are shown in figure 3. The red solid curve corresponds to √ s N N = 7 TeV, and the blue dashed curve is for √ s N N = 13 TeV. Since larger values of x correspond effectively to smaller values of the impact parameter b, where the suppression due to the strong interaction is stronger, S 2 (x) decreases with an increase of x. Also, the suppression somewhat increases with an increase of the invariant collision energy √ s N N as a result of the increase of σ tot pp (s) and the optical density Ω(s, b). For convenience, a simple fit to the curves in figure 3 is given in the appendix. Note that our values of S 2 (x) are consistent with the results for S 2 (x) for exclusive photoproduction of J/ψ and Υ mesons in pp UPCs [13] and also with the results of the calculation using a simpler model for the rapidity gap survival of ref. [53].

Results
We performed next-to-leading order (NLO) pQCD calculations implementing the inclusive k T -cluster algorithm [34] of the cross section of diffractive photoproduction of dijets in pp UPCs, eq. (2.1), using the following cuts (compare to the cuts used, e.g., in ref. [28]): x P ≤ 0.03 , z jets where E jet1,2 T and η jet1,2 are the transverse energies and the pseudorapidities of the two jets, respectively. For input, we used the DZ photon flux of the proton, eq. (2.9), modified by the rapidity gap survival probability S 2 (y), eq. (2.12), the GRV-HO photon PDFs [54], and the 2006 H1 proton diffractive PDFs (fit B) [43]. the cross section as a function of x jets γ , z jets P , E jet1 T , the invariant mass of the photon-proton system W , η jets = (η 1 + η 2 )/2, |∆η jets | = |η 1 − η 2 |, the invariant mass of the dijet system M 12 , and M X , see [28]. The central thick solid lines show the result of the calculation, when the renormalization and factorization scale µ is identified with the transverse energy of jet 1, µ = E jet1 T ; the dotted lines correspond to the calculation with µ = 2E jet1 T . Thus, the spread between the dashed lines quantifies the theoretical uncertainty of our NLO calculations associated with the choice of the factorization and renormalization scales. One can see from the figures that for our choice of E jet1 T > 20 GeV, this uncertainty is rather insignificant.

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Several features of the presented results merit discussion and comparison to diffractive dijet photoproduction in ep scattering at HERA [26][27][28]. First, the predicted yields are comparable to those observed in the ep case; the integrated cross section is O(hundreds pb) at √ s N N = 7 TeV and O(few nb) at √ s N N = 13 TeV. Second, while the general trends of the dependence on various variables are similar in the pp UPC and ep cases, the former allows to probe values of W exceeding those achieved in the ep case by at least a factor of ten and to produce dijets with the significantly larger M 12 and M X . In addition, the contribution of the low-z jets P region is much more important in the pp UPC case than in the ep case, which signals the enhanced sensitivity to the proton diffractive PDFs f D(4) b/p (x P , z P , t, µ 2 ) at small z P , where they are poorly constrained [42][43][44].
It is interesting to speculate that the large cross section of diffractive dijet photoproduction in pp UPCs at small z jets P might contribute to hard diffractive dijet production in pp scattering at large log 10 (x − P ) and cause the dependence of the suppression factor parametrizing the rapidity gap survival probability on the momentum fraction of the parton in the Pomeron [36,55].
In the experiment, to trigger on the events corresponding to diffractive dijet photoproduction in UPCs, one should employ the selection criteria typical for diffractive scattering in photoproduction: the absence of hadronic activity adjacent to the beam directions (presence of large rapidity gaps) will correspond to (very) small transverse momenta of the finalstate protons (ions) and guarantee that the exchanged photon is quasi-real and that the photon-target interaction is diffractive; the detector will register two hard jets with large p T and possibly the forward energy flow from the remnant diffractive final state (see figure 1).

General expression for the cross section
Taking one of the ions in figure 1 to be a nucleus and the other one to be the proton, the cross section of diffractive dijet photoproduction in pA UPCs reads (see eq. (2.1)): (3.1) The first term in eq. (3.1) corresponds to the process, when the photon flux is produced by the nucleus and the diffractive photoproduction of dijets takes place on the proton: ab→jets .

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nucleus: b/A is the diffractive PDF on a nucleus [56]; it a novel, yet unmeasured distribution. Note that the photon flux f γ/p (y) in eq. (3.3) corresponds to pA UPCs and includes the effect of the suppression of the strong photon-nucleus interaction at central impact parameters (see section 3.2).
It is important to point out that for most of the observables or in the case of the integrated cross section, the pA UPC cross section eq. (3.1) is dominated by the first term dσ(pA → A + 2jets + X + Y ) (+) . Indeed, while the photon flux of a nucleus scales as Z 2 , where Z is the nucleus charge, see, e.g. eq. (2.10), the diffractive PDFs of a nucleus after integration over the momentum transfer t scale only as A 4/3 in the impulse approximation; they are also further suppressed by nuclear shadowing [56]. Therefore, pA UPCs can be used to primarily study diffractive photoproduction of dijets on the proton by taking advantage of the dramatically enhanced intensity of the photon flux compared to pp UPCs. The same situation arises in exclusive photoproduction of J/ψ mesons in pA UPCs at the LHC at √ s N N = 5.02 TeV [9].

Flux of equivalent photons in pA UPCs
To calculate the photon flux in pA UPCs, one needs to take into account the suppression of the strong interaction between the colliding proton and the nucleus. The resulting photon flux of the ultrarelativistic nucleus reads, see e.g. [57]: where b is the impact parameter (the transverse distance between the centers of mass of the nucleus and the proton); Γ pA (b) is the probability to not have the strong pA interaction at the impact parameter b; and f γ/A (x, b) is the impact parameter dependent photon flux of the nucleus. The probability Γ pA (b) is given by the standard expression of the Glauber model for high-energy proton-nucleus scattering [58]: atomic mass number. In our analysis, we use the fit of ref. [52] for σ tot N N (s), the twoparameter Fermi model parametrization for ρ A (b, z) [59], and eq. (2.7) for f γ/A (x, b). In practice, the result of the full calculation can be approximated very well (with a few percent accuracy) by the photon flux of a point-like charge eq. (2.10) with b min = 1.15R A , where R A = 1.145A 1/3 ≈ 6.8 fm is the equivalent sharp radius of 208 Pb. The corresponding flux is given by the dotted curve labeled "PL", which is indistinguishable from the red solid curve. Note that since Γ pA (b) is a slow function of s N N in the considered energy range, it is a good approximation to use b min = 1.15R A both at √ s N N = 5.02 TeV and √ s N N = 8.16 TeV, the tentative Run-2 energy of pA collisions at the LHC.
The photon flux of the proton in pA UPCs can be found using eq. (3.4), where one replaces f γ/A (x, b) by f γ/p (x, b). The result is shown by the red solid curve labeled "FF+sup" in the right panel of figure 6. For comparison, the blue dot-dashed curve labeled "FF" shows the result, when one sets Γ pA = 1. Note that this curve coincides with the "DZ" and "PL" curves of figure 2 to a few percent accuracy. For convenience, in the appendix we give a simple analytic form of the factor of f sup p (x) parametrizing the difference between the "FF+sup" and "FF" curves shown in the right panel of figure 6. Note that f sup p (x) does not change when one increases √ s N N from √ s N N = 5.02 TeV to √ s N N = 8.16 TeV to better than a fraction of a percent accuracy. One can readily see from figure 6 that f γ/A (x) is larger than f γ/p (x) by approximately a factor of 5, 000 due to the Z 2 factor in eq. (2.7). This enhancement of the dσ(pA → A + 2jets + X + Y ) (+) term in eq. (3.2) wins over the nuclear enhancement of nuclear diffractive PDFs (see below) entering the dσ(pA → p + 2jets + X + Y ) (−) term. As a JHEP04(2016)158 result, the process, when the photon flux is produced by the nucleus, dominates the cross section of pA UPCs unless one probes very large values of W and η jets (see the results and discussion in section 3.4).

Nuclear diffractive PDFs
The nuclear diffractive PDFs f D(4) b/A (x P , z P , t, µ 2 ) entering the dσ(pA → p+2jets+X +Y ) (−) term in eq. (3.2) are conditional leading twist PDFs giving the distribution of a parton b in a nucleus in terms of the light-cone momentum fraction z P at the resolution scale µ, provided that the nucleus undergoes diffractive scattering characterized by the light-cone momentum fraction loss x P and the invariant momentum transfer squared t.
In the impulse approximation (IA), when the only nuclear effect is nuclear coherence, f where F A (t) is the nuclear form factor and t min = −(x P m p ) 2 /(1 − x P ) is the minimal momentum transfer. At high energies, the hard probe interacts coherently (simultaneously) with all nucleons of a nuclear target, which results in the effect of nuclear shadowing reducing nuclear PDFs compared to their IA expressions. In particular, the model of leading twist nuclear shadowing predicts a very significant suppression of nuclear diffractive PDFs [56], which can be quantified by the suppression factor of R b (x P , z P , µ 2 ): (3.7) Note that nuclear shadowing of nuclear diffractive PDFs breaks the phenomenological factorization eq. (2.4) of diffractive PDFs into the product of the "Pomeron" flux and PDFs of the "Pomeron". Predictions for R b (x P , z P , µ 2 ) [56] for sea quarks for the representative ranges of z P and x P and at µ 2 = 400 GeV 2 are shown in figure 7. An analysis reveals that R b (x P , z P , µ 2 ) very weakly depends on the parton flavor b, the scale µ, z P and x P (the latter is seen from figure 7). Therefore, in practical estimates, it is a good approximation to use the constant suppression factor:

Results
We theoretical uncertainty of our predictions associated with the choice of the renormalization and factorization scale. One can see from the figures that this uncertainty is not significant. A comparison of our predictions for pA UPCs shown in figures 8 and 9 to those for pp UPCs shown in figures 4 and 5 demonstrates that the general trends for the dependence of the cross section on various variables are similar in the pp and pA cases: very roughly, the pA results can be obtained from the pp ones by multiplying them by the scaling factor of (1/2)Z 2 (0.7 fm/R A ) ≈ 350, where took into account that the photon spectra of the proton and a nucleus extend up to x ∼ 1/b min = 1/(0.7 fm) and b min ∼ 1/R A , respectively, and that in the pA UPC cross section, the contribution of the minus-term in eq. (3.1) is generally small. Note that in the two upper panels of figures 8 and 9, the physical units along the y-axis are nb.
At the same time, there are marked differences between the pA and pp results. First, the cross section falls off faster as one increases E jet1 T or W in the pA case than in the pp case because the photon flux of a heavy ultrarelativistic nucleus decreases with an increase of the photon energy much faster than the photon flux of the proton. This also explains why at large values of E jet1 T and W , the cross section is dominated by the photon-fromproton contribution (the term dσ(pA → p + 2jets + X + Y ) (−) in eq. (3.1) corresponding to the photon flux emitted by the proton).
Second, unlike the symmetric η jets distribution in pp UPCs, this distribution is not symmetric in the case of pA UPCs. Indeed, at central and backward dijet rapidities, the dominant contribution to the cross section in eq. (3.1) comes from low-energy photons emitted by the nucleus. At the same time, forward dijet rapidities correspond to highenergy photons emitted by the nucleus, where the photon flux is very small, or to lowenergy photons emitted by the proton; the latter contribution dominates the cross section for sufficiently large positive η jets .
Note that without the effect of nuclear shadowing in nuclear diffractive PDFs, the photon-from-proton contribution (the red dot-dashed curves in figures 8 and 9) would be globally larger by a factor of 1/0.15 ≈ 7 (cf. eq. (3.8)), with a weak dependence on z P and x P (cf. figure 7).

General expression for the cross section
Considering nucleus-nucleus UPCs, we can readily write down the cross section of coherent diffractive dijet photoproduction (compare to eqs. (2.1) and (3.1)): Note that we considered the case of coherent nuclear scattering when both nuclei remain intact after either the photon emission or hard dijet photoproduction. By analogy with the pp and pA cases considered above, each term in eq.
For symmetric (equal beam-energy) AA UPCs that we consider in our work, the second and first terms in eq. (4.1) are related by a sign exchange of the dijet rapidities:

Flux of equivalent photons in AA UPCs
In the calculation of the photon flux produced by each ultrarelativistic nucleus in AA UPCs, one needs to suppress the strong nucleus-nucleus interaction. The resulting expression for the photon flux f γ/A (x) is is the impact parameter dependent photon flux of the nucleus (2.7) and Γ AA (b) is the probability for the nuclei to not interact strongly at the impact parameter b. It is given by the standard expression of the Glauber model for high-energy nucleus-nucleus scattering: An analysis shows that the result of the calculation of the photon flux using the exact expression of eq. (4.4) can be very well approximated by the much simpler expression for the photon flux produced by a relativistic point-like charge Z in eq. (2.10), when one uses b min ≈ 2R A for the minimal impact parameter, where R A is the equivalent sharp nucleus radius. Therefore, in our analysis of Pb-Pb UPCs at the LHC, we used eq.

Results
The One can see from these figures that the general trends of the dependence of the cross section of diffractive dijet photoproduction in AA UPCs resemble closely those already observed in the pp and pA and can be obtained approximately by simple rescaling. For instance, a comparison of the AA results at √ s N N = 5.1 TeV with the pA results at √ s N N = 8.16 TeV (corresponding to the same nucleus beam energy), one finds that the scaling factor between the distributions in the two cases is approximately A. In this estimate, we took into account that in the bulk of the considered kinematics, one has the approximate relation f j/p (x P , z P , µ 2 ) between the nucleus and proton diffractive PDFs, integrated over the momentum transfer t, (see eqs. (3.6)-(3.8)), and that the AA UPC cross section receives contributions of both nuclei, while the pA UPC cross section is dominated by the photon-from-nucleus contribution.
Note that the strong nuclear shadowing suppresses nuclear diffractive PDFs by the factor of 0.15, see eq.

JHEP04(2016)158 5 Factorization breaking in diffractive dijet photoproduction
It is well known from studies of diffractive photoproduction of dijets in ep scattering at HERA that collinear factorization for this process is broken, i.e., NLO pQCD calculations overestimate the measured cross sections by almost a factor of two [26][27][28][29][30][31][32][33][34]. However, the pattern of this factorization breaking remains unknown and presents one of the outstanding questions in this field: the data and the theory can be made consistent by introducing either the global suppression factor of R(glob.) ≈ 0.5 or the suppression factor of R(res.) ≈ 0.4 only for the resolved photon contribution. In addition, the HERA data on diffractive photoproduction of open charm [60] are in agreement with NLO pQCD calculations, which is consistent with diffractive QCD factorization. This agreement can be interpreted as an indication of absence of factorization breaking for the direct photon contribution and the charm-quark part of the resolved photon contribution to the dijet photoproduction cross section. Hence, it challenges the global suppression scenario of diffractive factorization breaking.
Factorization breaking in diffractive dijet photoproduction results from soft inelastic photon interactions with the proton (nucleus), which populate and thus partially destroy the final-state rapidity gap. Thus, it has exactly the same nature as the rapidity gap survival probability S 2 , which we discussed above in relation to pp UPCs, see eq. (2.12). At high energies, the photon interacts with protons and nuclei by fluctuating into various hadronic configurations (components) interacting with the target with different cross sections. Thus, it is natural to put forward the following physics scenario [61]: for the direct photon contribution, corresponding to weakly-interacting (point-like) fluctuations of the photon, factorization holds; for the resolved photon contribution corresponding to large-size photon fluctuations interacting with a typical vector meson-nucleon cross section, factorization is broken, which leads to the suppression factor of R(res.) ≈ 0.3 − 0.4. Note that beyond the leading order of pQCD, the separations of the direct and resolved contributions is ambiguous and depends on the factorization scheme and the factorization scale [32,38]; in the present work, we use the conventions of [34].
Our results presented so far in figures 4, 5, 8, 9, 11 and 12 assume no factorization breaking. Based on the observations and arguments summarized above, we will test the following two competing scenarios of diffractive QCD factorization breaking and implement them in our predictions for the cross section of diffractive dijet photoproduction: first, we assume the global suppression factor of R(glob.) = 0.5 for the proton target and R(glob.) = 0.1 for the nucleus target (the latter value is somewhat ad hoc, but reflects the important observation that it is much easier to break the nucleus than the proton, see figure 13 and its discussion below); second, we assume that the resolved photon contribution enters with the suppression factor of R(res.), while the direct photon contribution is unsuppressed. To estimate R(res.), we use the appropriate application of the two-state eikonal model of [51,62] (compare to eq. (2.12)):

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where T stands for the proton or nucleus target; V denotes the hadron-like fluctuation (component) of the photon, which is assumed to be represented by the ρ meson; A γT →V T (W, b) is the γT → V T amplitude in impact parameter space; P V T (W, b) is the probability to not have the strong inelastic vector meson-target interaction at the impact parameter b; and W is the invariant photon-nucleon energy.
For the proton target, we use where B(W ) is the slope of the t-dependence of the γp → ρp cross section. A fit to the available HERA data gives B(W ) = [11 + 0.5 ln(W/W 0 ) 2 ] GeV −2 , where W 0 = 72 GeV [63,64]. For the probability P V p (W, b), we use eqs. (2.13) and (2.14), where in the expression for the proton optical density, we substitute the total proton-proton cross section σ tot pp (s) by the ρ meson-nucleon cross section σ ρN (W ). Since we are interested in the large values of W > 100 GeV well beyond the HERA reach, we use in our analysis the following simple and conservative extrapolation: where W 0 = 100 GeV. The value of σ ρN (W ) at W = 100 GeV agrees with the analysis of ref. [25]. To find R(res.) for the nuclear target, we calculate A γA→V A (W, b) in eq. (5.1) using the Glauber model of nuclear shadowing for coherent photoproduction of vector mesons on nuclei in the high-energy limit, see e.g. [65]: where T A (b) is the nuclear optical density normalized to the number of nucleons A and f 2 V /(4π) = 2.01 is the photon-ρ meson coupling constant determined from the ρ → e + e − decay. Note that in eq. (5.4) we neglected the effect of the inelastic (Gribov) nuclear shadowing -at the large values of W that we consider, due to an eventual decrease of the dispersion of hadronic fluctuations of a projectile with an increase of energy [66], the relative importance of inelastic nuclear shadowing in our case is much smaller than that in the case of coherent ρ and φ photoproduction in AA UPCs [25,67].
For the suppression factor of P V A (W, b) in eq. (5.1), we use the standard Glauber model expression for the probability to not have the strong inelastic resolved photon (ρ meson)-nucleus interaction at the impact parameter b (compare to eq. (3.5)): For Pb, the values of R(res.) are an order of magnitude smaller, R(res.) ≈ 0.04, which reflects the very small probability of rapidity gap events with nuclear targets.
While our second scenario involving R(res.) captures the bulk of physics of diffractive factorization breaking coming from the hadron structure of the photon, it neglects such subtle points as the possible dependence of R(res.) on the parton flavor and x γ due to the separation of the resolved contribution into the point-like and hadronic terms, the hadronization corrections and bin migration effects, see the discussion in ref. [61]. Our aim here is to examine whether studies of diffractive dijet photoproduction in UPCs can help to distinguish between the two scenarios and, thus, to complement and extend the analysis of this process at HERA.
Note that for the first time, the issue of nuclear dependence of factorization breaking in diffractive dijet production in hard and ultraperipheral pA scattering was considered in [68]. It was found that soft inelastic proton-nucleus interactions significantly suppress the rapidity gap probability in hard pA scattering, which is in line with the small values of R(glob.) and R(res.) for the nucleus target, which we use in our analysis.
The resulting cross sections of diffractive dijet photoproduction in pp, pA and AA UPC are presented in figure [14][15][16][17][18][19]. The red solid lines correspond to the global suppression factor of R(glob.) = 0.5 for the proton target and R(glob.) = 0.1 for the nucleus target (note that in the case of pA UPCs, we encounter a mixed situation); the blue dot-dashed lines correspond to the suppression of the resolved photon contribution only: R(res.) = 0.4 for the diffracting proton (pp and the photon-from-nucleus contribution to pA) and R(res.) = 0.04 for the diffracting nucleus (the photon-from-proton contribution to pA and AA). For comparison, we also show our results that do not include the effect of diffractive QCD factorization breaking by black dotted lines labeled "R = 1". Note that in all cases, we show only the predictions corresponding to the central value of the renormalization and factorization scale µ = E jet1 T . As one observes, the most sensitive variable to distinguish global from resolved-only suppression is x jets γ as expected, where resolved-only suppression is smaller in the highest

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and larger in the lower bins. As also observed previously in diffractive dijet photoproduction at HERA [32], the distributions in E jet1 T also show differences, i.e. resolved-only suppression results in harder spectra than global suppression. These differences are more pronounced in pA collisions compared to pp collisions due to the enhanced photon flux and asymmetric experimental setup. In pA UPCs, also the z jets P distributions differ, i.e. resolved-only suppression is less effective at small values of that variable, which are correlated with large x jets γ . Naturally, similar differences are then observed in the average rapidity and rapidity difference distributions, from which the observed momentum fraction variables are derived. In pA UPCs, the differences of the two suppression schemes are furthermore enhanced at higher center-of-mass energy, where the low z jets P region is particularly enhanced. In contrast, in AA collisions the shape of the z P distribution is quite different from those in pp and pA collisions, but is similar in the two used suppression schemes, which makes it less sensitive to the factorization breaking pattern.

Conclusions
For the first time, using NLO pQCD, we make predictions for the cross sections of diffractive dijet photoproduction in pp, pA and AA UPCs in the kinematics of Runs 1 and 2 at the LHC. Using general kinematic conditions and cuts on the final state, we found that the values of the cross section as a function of various variables are sufficiently large, i.e., this process can be observed. Compared to studies of this process in ep scattering at HERA, we observe that UPCs provide an enhanced sensitivity to the low-z jets P region probing the quark and gluon diffractive parton distributions in the proton and nuclei at small momentum fractions z and an access to much larger values of W .
In our calculations, we used nuclear diffractive PDFs, which are strongly suppressed by nuclear shadowing; neglecting this effect, our predictions for AA UPCs and for the photon-nucleus contribution to pA UPCs would be larger by the factor of seven.
UPCs also give a new handle on the issue of diffractive QCD factorization breaking through its A dependence: while the two competing schemes of factorization breaking based on the global and resolved-only suppression factors give rather similar predictions for pp UPCs (like in the case of ep scattering at HERA), the two scenarios give rather different predictions for AA UPCs and to some extent for pA UPCs. The best observable to look for this effect is the x jets γ dependence at large x jets γ , which is dominated by the direct photon contribution and where the ordering between the cross sections calculated using R(glob.) and R(res.) changes. This is illustrated in figure 20 summarizing our results for the x jets γ dependence in Run 1 (upper panel) and Run 2 (lower panel). Note that in this figure, the two schemes of factorization breaking for the pp case are indistinguishable.
The results presented in this work are based on the NLO collinear factorization formalism of pQCD. In the framework of high-energy QCD, diffractive dijet production in photon-proton and photon-nucleus collisions was considered in the Color Glass Condensate (CGC) formalism at leading order in ref. [69]. It was found that the effects of gluon saturation can be searched for in the dijet azimuthal angle correlations and t distributions. In addition, a theoretical framework for diffractive production of jets in the QCD       shock-wave approach has started to be developed in a series of papers [70,71]. It will be interesting to confront these different approaches with LHC data in the future.

A Suppression factors used for calculations in this paper
For convenience of the reader, we give in this appendix simple parametrizations of the various suppression factors used in our calculations in this paper.
1. The rapidity gap survival probability factor of S 2 (x) for pp UPCs, which is given by eq. (2.12) and shown in figure 3, can be fitted to better than 5% accuracy by the following simple form: The last equality gives a simple fit, which reproduces the calculation of f sup p to better than 5% accuracy. Note that f sup p (x) gives the ratio of the red solid and the blue dot-dashed curves in the right panel of figure 6. The fit of eq. (A.2) is valid both at √ s N N = 5.02 TeV and √ s N N = 8. 16 TeV, since f sup p (x) does not change in this energy interval to better than a fraction of a percent accuracy.
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