# Next-to-Leading-Order QCD corrections to production at the LHC

## Abstract

In this work, we calculate the next-to-leading-order (NLO) QCD corrections to the process via the color-singlet mechanism at the LHC. The results show that the partial cross section (3GeV and 3) is enhanced by a factor of about 2.0, and the differential cross section can be enhanced by two orders of magnitude in the large transverse momentum region of . Furthermore, the polarization of changes from transverse polarization at leading-order to longitudinal polarization at NLO. For the inclusive hadroproduction, it is known that the color-octet contributions are one order of magnitude larger than the color-singlet contribution, and the polarization distribution is dominated by the color-octet behavior at NLO. In contrast, for production the color-singlet contribution is of the same order as the color-octet contribution, and the polarization distribution arises from both the color-singlet and color-octet. Therefore, measurements of production associated with a direct photon at the hadron collider could be an important supplement to testify the theoretical framework treating with the heavy quarkonium. In addition, an NLO QCD correction to production at the LHC is also presented in this paper.

###### pacs:

12.38.Bx, 13.25.Gv, 13.60.LeFor a long time, the productions and decays of heavy quarkonium have been an ideal laboratory to investigate quantum chromodynamics. The large mass of the heavy quarks provides a large scale for production and decay processes. This large scale makes the factorization of the calculations for these processes available, and the hard part in the calculations can be calculated perturbatively. Conventionally, the color-singlet mechanism(CSM) Einhorn and Ellis (1975) was used to describe the production and decay of heavy quarkonium. However, the CSM has encountered many difficulties in various theoreticalBarbieri et al. (1976) and experimental aspectsAbe et al. (1992). In 1995, non-relativistic quantum chromodynamics(NRQCD) was put forwardBodwin et al. (1995). By including the contributions from the high Fock states, NRQCD can overcome the theoretical difficultiesBodwin et al. (1992). At the same time, the NRQCD predictions are consistent with experimental dataBraaten and Yuan (1994). Although NRQCD has had many successes, there are also many problems in the production of heavy quarkoniumBrambilla et al. (2004).

In 1995, Kramer calculated the NLO QCD corrections to inclusive photoproduction and found that the data from HERA could be understood by just including the high order QCD corrections in CSM Kramer (1996). Recently, many studies Zhang et al. (2006); Gong and Wang (2008a) have shown that NLO QCD corrections in CSM to related production processes at B-factory change the theoretical predictions dramatically. Furthermore, at the Tevatron, the NLO QCD corrections in CSM enhance the total cross section by a factor of 2 and give large values for the transverse momentum distribution of , especially in the large regionCampbell et al. (2007); Gong and Wang (2008c). The polarization status of drastically changes from transverse-polarization dominant at leading-order (LO) into longitudinal-polarization dominant at NLO for hadroproductionGong and Wang (2008c, d). Artoisenet and his collaborators suggested that the distribution of at the Tevatron can be interpreted in the CSM by taking the NNLO real part into account Artoisenet et al. (2008). It is quite clear that higher order QCD corrections play a very important role in theoretical predictions for the production of heavy quarkonium, and their effects should be carefully investigated in all the relevant processes.

In the framework of CSM, the associated production of at a hadron collider was first proposed as a good channel to investigate the gluon distribution in the proton with a relatively clean signalDrees and Kim (1992). Soon thereafter, it was used to study the polarized gluon distributionDoncheski and Kim (1994) and the production mechanism of heavy quarkoniumKim and Mirkes (1995). In reference Roy and Sridhar (1995), the associated production of at the Tevatron has been considered in the CSM at the LO, and the results show that the contribution from gluon fusion process is dominant over that from the fragmentation processes. Kim investigated the contribution of color-octet processes to the hadroproduction of and found that the color-octet contributions are dominant in the large regionKim et al. (1997). The contribution from fragmentation processes is smaller than the fusion contribution within the NRQCD framework at the LHCMathews et al. (1999). In reference Kniehl et al. (2002), the authors obtained a theoretical prediction for hadroproduction at the hadron collider, and the numerical results show that the transverse momentum distribution of production is smaller in the CSM than that in the color-octet mechanism (COM) in the large region at LO. To further study the effect of the NLO QCD corrections on heavy quarkonium hadroproduction, in this paper we calculate the NLO QCD corrections to hadroproduction at the LHC and present theoretical predictions for the distribution of the production and polarization for .

We employ the automated Feynman Diagram Calculation package (FDC) to perform the analytic evaluation of all the processes. FDC is a powerful program based on the LISP language designed to automate the NLO calculation and was initially developed by WangWang (2004). Its one-loop part was recently completed by Wang and Gong Gong and Wang (2008e). It has recently been successfully applied to several quarkonium production processes Gong and Wang (2008a, c, d); Gong et al. (2008a, b).

For the process at LO, only the gluon fusion process contributes at the partonic level with six Feynman diagrams, which is similar to that of in inclusive hadroproduction. The LO total cross section is obtained by convoluting the partonic cross section with the parton distribution function (PDF) in the proton:

(1) |

where is the factorization scale. In the following, represents the corresponding partonic cross section.

When the cross section is expanded to NLO on , the coupling constant of quantum chromodynamics, there are one virtual correction and three real correction processes. They are listed as the following:

(2) | |||

(3) | |||

(4) | |||

(5) |

In calculating the virtual corrections in Eq.(2), there are 111 Feynman diagrams at NLO. The ultraviolet (UV) and infrared (IR) singularities are normalized and separated by using the dimensional regularization. Furthermore, the same renormalization scheme as in Ref. Gong and Wang (2008c, d) is applied to redefine the quark mass, coupling constant and the quark or gluon fields, and then the renormalized amplitude without UV singularities is obtained. The Coulomb singularity, which comes from the diagrams with a virtual gluon connecting the quark and anti-quark pair in , is regulated by introducing a small relative velocity between the quark and anti-quark pair and is absorbed into the redefinition of the wave function of . Therefore, the one-loop amplitude is free of UV and Coulomb singularities and the virtual corrections to the NLO cross section are expressed as

(6) |

where is the amplitude at LO. It is UV and Coulomb finite, but has IR singularities. To obtain an infrared-safe cross section, it is needed to cancel the IR singularities by adding the contributions from real processes at NLO.

For the real processes in Eqs.(3), (4) and (5), there are IR singularities in the phase space integration which are divided into soft and collinear singularities. The soft singularity is from a soft gluon emitting from the initial gluons. The collinear singularity is from the initial gluon (or quark) emitting a gluon which is nearly parallel to the parent particle. It is easy to find that soft singularities caused by emitting soft gluons from the charm quark-antiquark pair in are canceled by each other. Using the standard two cut-off slicing methodHarris and Owens (2002), we decompose the phase space into three regions by introducing two small cutoffs and . Therefore, convoluting the parton level cross section with the parton distribution function, the cross section of the real processes is represented as

(7) |

Here is the contribution from the hard noncollinear part of the phase space that is IR finite, is the soft part and is the hard collinear part. After absorbing the mass factorization parts into the PDFs, there is a finite term remaining which is similar to that in Eq.(43) in Ref.Gong and Wang (2008d). By adding all the contributions together, a finite total cross section is obtained.

The polarization of is an important physical measurement to identify different production mechanisms. Therefore, the polarization is calculated at NLO. Here we describe the decay of in its rest frame with the 3-momentum direction of as the z-axis. The polarization parameter is defined as

(8) |

where and are the cross sections of transversely and longitudinally polarized respectively. corresponds to fully longitudinal polarization and to fully transverse polarization.

To check the gauge invariance for each subprocess, the polarization vectors are replaced by the corresponding momentum in the numerical calculation and the gauge invariance is obviously observed at double precision level. Since the two phase space cutoffs are chosen to handle the IR singularities of the real processes, we varied the cutoffs by a few orders of magnitude to numerically check the independence of the results from the cutoffs and obtained consistent results within the error tolerance.

In the numerical calculation, we use =1/137, =1.5GeV, and . From the leptonic width of , the wave function at the origin is extracted by

(9) |

We obtain =0.944GeV at , keV. The Cteq6L1 and Cteq6MPumplin et al. (2002) are used in the calculations at LO and NLO respectively, with the corresponding running formula in Cteq6 being used. The renormalization scale and the factorization scale are set to . The center-of-mass energy at the LHC is 14TeV and the rapidity cuts for both and the direct photon are chosen as . Because the perturbative expansion does not work well in the small transverse momentum region and the large rapidity region, we impose and cuts on the numerical calculation. In these processes, the direct photon has nothing to do with the infrared singular structure, so it can be identified with any experimentally acceptable kinematic cuts. Our numerical calculation is obviously consistent with this expectation. Of course, the cut conditions imposed on the direct photon will affect the numerical results. In the following, we fix the rapidity cut of the photon as and vary its cuts to calculate the numerical results.

By replacing the corresponding parameters as

(10) |

the results of can be obtained. For the bottom quark mass and the wave function of at the origin, =4.75GeV and =7.74GeV are used. We use the Eq.(9) to calculate the with and keV.

The distribution of with different cut conditions on the associated photon is shown in Fig. 1. It is noteworthy that there are two cut conditions, of which one is the cut condition and the other is the associated photon cut condition since both and the associated photon have to be measured experimentally. The NLO numerical results of the distribution of are larger than the LO results by orders of magnitude in the large region, and different cut conditions only affect the results in the region near the minimum endpoint in . In the case of inclusive hadroproduction at NLO in COM Gong et al. (2008a), the results show that the NLO QCD corrections change the results by about 10 percent. Therefore, we can expect that the NLO QCD corrections will modify the results of at NLO in COM slightly, since the process is quite similar to inclusive hadroproduction at NLO in COM. Fig. 2 shows that the NLO QCD corrections also change the distribution of , but with less enhancement than that of .

The theoretical predictions of the polarization at NLO are presented in Fig. 3 with different cut conditions. They are similar to the result of inclusive hadroproduction. The polarization drastically changes from the more transverse polarization at LO to a more longitudinal polarization at NLO. Also, the polarization parameter of at NLO becomes closer to -0.9 as increases. In the figures, the different curves are plotted with different cut conditions. It is clear that the cut condition for the associated photon has a greater effect near the minimum endpoint of and a smaller effect in the large region. From Fig. 4, the polarization of also changes from transverse-polarization dominant to longitudinal-polarization dominant, and at NLO becomes closer to -0.8 as increase. In the small region, the convergence of the numerical calculation becomes worse, and it requires too much CPU time to improve the precision of the calculations. At the same time, the denominator of changes its sign in the neighborhood of a point in the small region, meaning that the value of undergoes a vast change around that point. The small value of the denominator also amplifies the error in the calculation, indicating that the convergence of the perturbative expansion is bad and that higher order contributions are important in the small region, especially for the distribution of the polarization parameter . Therefore, the small region is further discarded in our presentation of .

In Fig. 5, the dependence of the partial cross section (3GeV,) for production at LO and NLO are shown with our default choice, . In other words, the factorization scale equals to the renormalization scale, and ranges from to . There is no cut for the associated photon. It is obvious that QCD corrections reduce the dependence of the partial cross section for production and moderate the dependence for production.

To illustrate the influence of the cut conditions on the partial cross section, we present LO and NLO partial cross sections for production at the LHC with different cut conditions in Table 1. In Fig. 6, we plot the dependence of the partial cross section on the cut of the direct photon with the cut of fixed at 10GeV. The plots show that the contributions from small photon are large and the partial cross section decreases as the cut on the photon increases. For the production of , when the cut on the photon becomes too close to the cut of , the partial cross section decreases rapidly and the influence of the error becomes severe. In this case, too many contributions from the real processes are cut off and the perturbative calculation becomes worse. Therefore, the partial cross section cannot be taken seriously when the cut condition of the photon approaches the cut condition of .

In summary, we have calculated NLO QCD corrections to the production of associated with a direct photon at the LHC in CSM. For production, the partial cross section is enhanced by a factor of about 2.0 with transverse momentum cut 3GeV and rapidity cut for both and the direct photon. The transverse momentum distribution of at NLO is enhanced by orders of magnitude over LO calculations as becomes larger. The polarization is calculated, and the results show that the polarization drastically changes from transverse-polarization dominant at LO to longitudinal-polarization dominant at NLO. The situation is quite similar to the case of NLO QCD corrections to the inclusive hadroproduction. It can be seen that NLO results on hadroproduction in CSM is of the same order of magnitude as LO results in COMKim et al. (1997); Kniehl et al. (2002). As a reasonable estimate from the experience of NLO QCD correction calculation to inclusive hadroproduction in COMGong et al. (2008a), the NLO distribution for hadroproduction in COM will be changed slightly and the polarization will remain almost the same. Therefore, the results of production associated with a direct photon from the CSM and COM are of the same order of magnitude at NLO. Therefore, the polarization measurement would be able to distinguish the contributions from the CSM and COM since the theoretical predictions of polarization are obviously different for the CSM and COM. In contrast to the case of inclusive hadroproduction, the NLO result of CSM is about one order of magnitude smaller than the NLO result of COM, and so there is no way for the CSM part to play an important role in the final polarization distribution.

To measure the production of associated with a direct photon at the LHC, the direct photon must be identified. To cut the enormous background of photons emitted in jet hadronization, photons from jets are attributed to the jets and a direct photon, which is isolated from any jets, should be identified. Therefore, being quite different from inclusive hadroproduction, the hadroproduction of associated with a direct photon will be an important process to investigate the production mechanism of heavy quarkonium and impose new constraints on the contribution of COM to heavy quarkonium hadroproduction.

We thank Gong Bin for helpful discussions. This work is supported by the National Natural Science Foundation of China (No. 10775141) and by the Chinese Academy of Sciences under Project No. KJCX3-SYW-N2.

### References

- M. B. Einhorn and S. D. Ellis, Phys. Rev. D12, 2007 (1975); S. D. Ellis, M. B. Einhorn, and C. Quigg, Phys. Rev. Lett. 36, 1263 (1976); C.-H. Chang, Nucl. Phys. B172, 425 (1980); E. L. Berger and D. L. Jones, Phys. Rev. D23, 1521 (1981); R. Baier and R. Ruckl, Nucl. Phys. B201, 1 (1982).
- R. Barbieri, R. Gatto, and E. Remiddi, Phys. Lett. B61, 465 (1976); R. Barbieri, M. Caffo, R. Gatto, and E. Remiddi, Phys. Lett. B95, 93 (1980); R. Barbieri, M. Caffo, R. Gatto, and E. Remiddi, Nucl. Phys. B192, 61 (1981); R. Barbieri, E. d’Emilio, G. Curci, and E. Remiddi, Nucl. Phys. B154, 535 (1979); K. Hagiwara, C. B. Kim, and T. Yoshino, Nucl. Phys. B177, 461 (1981); P. B. Mackenzie and G. P. Lepage, Phys. Rev. Lett. 47, 1244 (1981).
- F. Abe et al. (CDF), Phys. Rev. Lett. 69, 3704 (1992); F. Abe et al. (CDF), Phys. Rev. Lett. 71, 2537 (1993).
- G. T. Bodwin, E. Braaten, and G. P. Lepage, Phys. Rev. D51, 1125 (1995), eprint hep-ph/9407339.
- G. T. Bodwin, E. Braaten, and G. P. Lepage, Phys. Rev. D46, 1914 (1992), eprint hep-lat/9205006.
- E. Braaten and T. C. Yuan, Phys. Rev. D50, 3176 (1994), eprint hep-ph/9403401; E. Braaten and S. Fleming, Phys. Rev. Lett. 74, 3327 (1995), eprint hep-ph/9411365; P. L. Cho and A. K. Leibovich, Phys. Rev. D53, 150 (1996a), eprint hep-ph/9505329; P. L. Cho and A. K. Leibovich, Phys. Rev. D53, 6203 (1996b), eprint hep-ph/9511315.
- N. Brambilla et al. (Quarkonium Working Group) (2004), eprint hep-ph/0412158; J. P. Lansberg, Int. J. Mod. Phys. A21, 3857 (2006), eprint hep-ph/0602091; X.-Q. Li, X. Liu, and Z.-T. Wei (2008), eprint 0808.2587.
- M. Kramer, Nucl. Phys. B459, 3 (1996), eprint hep-ph/9508409; M. Kramer, Prog. Part. Nucl. Phys. 47, 141 (2001), eprint hep-ph/0106120.
- Y.-J. Zhang, Y.-j. Gao, and K.-T. Chao, Phys. Rev. Lett. 96, 092001 (2006), eprint hep-ph/0506076; Y.-J. Zhang and K.-T. Chao, Phys. Rev. Lett. 98, 092003 (2007), eprint hep-ph/0611086; Y.-J. Zhang, Y.-Q. Ma, and K.-T. Chao, Phys. Rev. D78, 054006 (2008), eprint 0802.3655.
- B. Gong and J.-X. Wang, Phys. Rev. D77, 054028 (2008a), eprint 0712.4220; B. Gong and J.-X. Wang, Phys. Rev. Lett. 100, 181803 (2008b), eprint 0801.0648.
- J. Campbell, F. Maltoni, and F. Tramontano, Phys. Rev. Lett. 98, 252002 (2007), eprint hep-ph/0703113.
- B. Gong and J.-X. Wang, Phys. Rev. Lett. 100, 232001 (2008c), eprint 0802.3727.
- B. Gong and J.-X. Wang, Phys. Rev. D78, 074011 (2008d), eprint 0805.2469.
- P. Artoisenet, J. Campbell, J. P. Lansberg, F. Maltoni, and F. Tramontano, Phys. Rev. Lett. 101, 152001 (2008), eprint 0806.3282.
- M. Drees and C. S. Kim, Z. Phys. C53, 673 (1992).
- M. A. Doncheski and C. S. Kim, Phys. Rev. D49, 4463 (1994), eprint hep-ph/9303248.
- C. S. Kim and E. Mirkes, Phys. Rev. D51, 3340 (1995), eprint hep-ph/9407318; E. Mirkes and C. S. Kim, Phys. Lett. B346, 124 (1995), eprint hep-ph/9504412.
- D. P. Roy and K. Sridhar, Phys. Lett. B341, 413 (1995), eprint hep-ph/9407390.
- C. S. Kim, J. Lee, and H. S. Song, Phys. Rev. D55, 5429 (1997), eprint hep-ph/9610294.
- P. Mathews, K. Sridhar, and R. Basu, Phys. Rev. D60, 014009 (1999), eprint hep-ph/9901276.
- B. A. Kniehl, C. P. Palisoc, and L. Zwirner, Phys. Rev. D66, 114002 (2002), eprint hep-ph/0208104.
- J.-X. Wang, Nucl. Instrum. Meth. A534, 241 (2004), eprint hep-ph/0407058.
- B. Gong and J.-X. Wang (2008e), eprint in preparation.
- B. Gong, X. Q. Li, and J.-X. Wang (2008a), eprint 0805.4751.
- B. Gong, Y. Jia, and J.-X. Wang (2008b), eprint 0808.1034.
- B. W. Harris and J. F. Owens, Phys. Rev. D65, 094032 (2002), eprint hep-ph/0102128.
- J. Pumplin et al., JHEP 07, 012 (2002), eprint hep-ph/0201195.