The Integrand Reduction of One and TwoLoop Scattering Amplitudes
Abstract
The integrandlevel methods for the reduction of scattering amplitudes are wellestablished techniques, which have already proven their effectiveness in several applications at oneloop. In addition to the automation and refinement of tools for oneloop calculations, during the past year we observed very interesting progress in developing new techniques for amplitudes at two and higherloops, based on similar principles. In this presentation, we review the main features of integrandlevel approaches with a particular focus on algebraic techniques, such as Laurent series expansion which we used to improve the oneloop reduction, and multivariate polynomial division which unveils the structure of multiloop amplitudes.
The Integrand Reduction of One and TwoLoop Scattering Amplitudes
\abstract@cs
1 Overview
Scattering amplitudes are analytic functions of the momenta of the particles involved and they can be studied by exploring their singularity structure [1, 2]. The investigation of the residues at the poles, which correspond to particles going on their massshell, led to the discovery of new important relations. The BCFW recurrence relation [3], its link to the leading singularity of oneloop amplitudes [4], and the OPP integranddecomposition formula for oneloop integrals [5] have shown the underlying simplicity beneath the rich mathematical structure of quantum field theory. Moreover they provided the theoretical framework to develop efficient computational techniques at the nexttoleading order in perturbation theory [6, 7, 8, 9, 10, 11, 12, 13].
The integrand reduction methods, originally developed for oneloop diagrams [5], use the singularity structure of the integrands to decompose the (integrated) amplitudes in terms of Master Integrals (MI’s). The multiparticle pole expansion of the integrand is equivalent to the decomposition of the numerator in terms of products of denominators, multiplied by polynomials which correspond to the residues at the multiplecuts.
The parametric form of the polynomial residues is processindependent and can be determined once and for all from the structure of the corresponding multiple cut. The actual value of the coefficients which appear in the residues is instead processdependent and, in the framework of the integrandreduction their determination is achieved by polynomial fitting, through the evaluation of the (known) integrand at values of the loopmomenta fulfilling the cut conditions [14].
Extensions of the integrand reduction method beyond oneloop, first proposed in [14, 15], have been systematized within the mathematical framework of multivariate polynomial division and basic principles of algebraic geometry [16, 17]. Recently they become the target of several new developments [18, 19, 20], thus giving birth to a new direction in the study of multiloop amplitudes. An alternative approach to twoloop calculations based on maximal unitarity has been pursued in [21, 22, 23, 24].
2 Automation of OneLoop Calculations
The continuous improvement of new techniques for oneloop computations led to tremendous progress in the field of NLO QCD corrections [25]. Calculations of increasing complexity have been performed with improved algebraic reduction methods based on Feynmandiagrammatic algorithms, as well as with new numerical techniques based on the idea of reconstructing oneloop amplitudes from their unitarity cuts. These theoretical developments found an ideal counterpart in the integrandlevel reduction algorithm.
The GoSam framework [10, 26] combines the automated algebraic generation of dimensional unintegrated amplitudes obtained via Feynman diagrams, with the numerical integrandlevel reduction. Concerning the reduction, GoSam allows to choose at runtime (namely without regenerating the code) among integrandlevel dimensional reduction [5, 27], as implemented in Samurai [28], or traditional tensor reduction interfaced through tensorial reconstruction [29, 30]. The coefficients determined by the reduction are then multiplied by the corresponding scalar (master) integrals [31]. Recent examples of full NLO QCD calculations performed within this framework include [32] and jet [33] at the LHC.
3 IntegrandReduction via Laurent Expansion
An improved version of integrandreduction method for oneloop amplitudes was presented in [34], elaborating on the the techniques proposed in [35, 36]. This method allows, whenever the analytic form of the numerator is known, to extract the unknown coefficients of the integrand decomposition by performing a Laurent expansion.
In general, the multiplecut conditions constrain the loop momentum. Therefore, the onshell solutions are parametrized by those components which are not completely determined in terms of the external kinematics.
The original reduction algorithm [37, 38, 28] requires, in these cases: to sample the numerator on a finite subset solutions; to subtract from the integrand all the nonvanishing contributions coming from higherpoint residues; and finally to solve a linear system of equations in order to find the value of the unknown coefficients parametrizing the residue of the cut.
This algorithm can be simplified by exploiting the knowledge of the analytic expression of the integrand. Indeed, by performing a Laurent expansion with respect to one of the free parameters which appear in the solutions of the cut, both the integrand and the subtraction terms exhibit the same polynomial behavior of the residue. Moreover, the contributions coming from the subtraction terms can be implemented as corrections at the coefficient level, hence replacing the subtractions at the integrand level of the original algorithm. The parametric form of this corrections can be computed once and for all, in terms of a subset of the higherpoint coefficients. With this method the number of coefficients entering in each subtraction term is significantly reduced. For instance, box and pentagons do not affect at all the computation of lowerpoints coefficients.
In summary, this method identifies the coefficients of a residue with the ones of the Laurent expansion of the numerator (with respect to one of the free components of the loop momentum which are not fixed by the cut conditions). The result must be corrected by a subtraction term which is a known function of the higher point coefficients. If either the analytic expression of the integrand or the tensor structure of the numerator is known, this procedure can also be implemented in a seminumerical algorithm. Indeed, the coefficients of the Laurent expansion of a rational function can be computed, either analytically or numerically, by performing a polynomial division between the numerator and the denominator. This method has been implemented in a c++ library, and preliminary tests show an improvement in the computational performance with respect to the standard algorithm.
4 Higherrank integrands
The integrand decomposition was originally developed for renormalizable gauge theories, where, at oneloop, the rank of the numerator cannot be greater than the number of external legs . In [34], we extended the decomposition to the case where the rank becomes larger than . This extension is required, for instance, for applying the integrand reduction to the production of Higgs in combination with jets, in the gluonfusion channel via effectivegluon vertex, generated by the large topmass limit. As a first step along this direction, we implemented within Samurai the extension of the polynomial residues and the corresponding additional sampling required to fit their coefficients.
5 IntegrandReduction for TwoLoop Scattering Amplitudes and beyond
The first extension of the integrand reduction method beyond oneloop was proposed in [14]. A key point of the higherloop extension is the proper parametrization of the residues at the multiparticle poles. We define irreducible scalar products (ISP’s) the set of scalar products, among the loop momenta and either external momenta or polarization vectors constructed out of them, which cannot be expressed in terms of denominators. Residues at the multiparticle poles can be written as a multivariate polynomial in the ISP’s. Hence, a systematic classification of the polynomial structures of the residues is mandatory.
This task has been successfully achieved in [17], where we have shown that the shape of the residues is uniquely determined by the onshell conditions alone, without any additional constraint. We have derived a simple integrand recurrence relation that generates the required multiparticle pole decomposition for arbitrary amplitudes, independently of the number of loops. The algorithm presented in [17] relies on general properties of the loop integrands
(5.0) 

When the number of denominators is larger than the total number of the components of the loop momenta, the weak Nullstellensatz theorem yields the trivial reduction of an denominator integrand in terms integrands with denominators.

When is equal or less than the total number of components of the loop momenta, we divide the numerator modulo the Gröbner basis of the ple cut, namely modulo a set of polynomials vanishing on the same onshell solutions as the cut denominators. The remainder of the division is the residue of the ple cut. The quotients generate integrands with denominators which should undergo the same decomposition.
This allows us to cast the each numerator , sitting on a set of denominators , in the form
(5.0) which inserted in the expression for the generic the denominator integrand, provides the aforementioned recurrence relation
(5.0) We remark that the procedure, together with Eqs.(5) and (5), hold for any number of loops and in all dimensions.

By iteration, we extract the polynomial forms of all residues. The algorithm will stop when all cuts are exhausted, and no denominator is left, leaving us with the complete integrand reduction formula.
In [17], we have also proved a theorem on the maximumcuts, i.e. the cuts defined by the maximum number of onshell conditions which can be simultaneously satisfied by the loop momenta. The onshell conditions of a maximum cut lead to a zerodimensional system. The Finiteness Theorem and the Shape Lemma ensure that the residue at the maximumcut is parametrized by coefficients, where is the number of solutions of the multiple cutconditions. This guarantees that the corresponding residue can always be reconstructed by evaluating the numerator at the solutions of the cut. The maximum cut theorem generalizes at any loop the simplicity of the oneloop quadruplecut [4, 5], where the only two solutions of the cut univocally determine the two coefficients needed to parametrize the residue.
As a first application, we applied the algorithm to a generic oneloop integrand, reproducing the wellknown dimensional integrand decomposition formula [5, 27]. Very recently [39], we have applied our algorithm to the twoloop fivepoint planar and nonplanar amplitudes in Super YangMills (SYM) and Supergravity (SUGRA). The numerators of the integrals have at most rank two in the integration momenta. In particular we perform the integrand reduction both seminumerically, by polynomial fitting, and analytically. The latter computation has been performed generalizing the method of integrand reduction through Laurent expansion [34] discussed above.
6 Conclusions
The integrand reduction methods, which use the singularity structure of the integrands to decompose the (integrated) amplitudes in terms of Master Integrals, already proved their effectiveness in applications at the oneloop level. Several efforts are under way in order to extend this formalism to higher orders, starting with twoloop amplitudes.
We recently proposed a new approach for the reduction of scattering amplitudes, based on multivariate polynomial division. This technique yields the complete integrand decomposition for arbitrary amplitudes, regardless of the number of loops. We have shown that the shape of the residues is uniquely determined by the onshell conditions, and we have derived a simple integrand recurrence relation that generates the multiparticle pole decomposition for arbitrary multiloop amplitudes. We have successfully applied the new reduction algorithm to oneloop and twoloop examples.
The method is well suited for a numerical implementation, but it also allows for the extraction of full analytic results, thus providing a universal and powerful tool for the generalization of integrandlevel reduction techniques to all orders in perturbation theory.
Acknowledgments
P.M., T.P., and H.v.D. are supported by the Alexander von Humboldt Foundation, in the framework of the Sofja Kovaleskaja Award, endowed by the German Federal Ministry of Education and Research. The work of G.O. is supported in part by the National Science Foundation under Grant No. PHY1068550 and PSCCUNY Award No. 6518800 43.
References
 [1] Z. Bern, L. J. Dixon, D. C. Dunbar and D. A. Kosower, Nucl. Phys. B 425 (1994) 217.
 [2] F. Cachazo, P. Svrcek and E. Witten, JHEP 0409 (2004) 006.
 [3] R. Britto, F. Cachazo and B. Feng, Nucl. Phys. B 715 (2005) 499.
 [4] R. Britto, F. Cachazo and B. Feng, Nucl. Phys. B 725 (2005) 275.

[5]
G. Ossola, C. G. Papadopoulos and R. Pittau,
Nucl. Phys. B 763 (2007) 147;
G. Ossola, C. G. Papadopoulos and R. Pittau, JHEP 0707 (2007) 085;
G. Ossola, C. G. Papadopoulos and R. Pittau, JHEP 0805 (2008) 004.  [6] C. F. Berger et al., Phys. Rev. D 78 (2008) 036003.
 [7] W. T. Giele and G. Zanderighi, JHEP 0806 (2008) 038.
 [8] G. Bevilacqua et al.,arXiv:1110.1499 [hepph].
 [9] V. Hirschi et al., JHEP 1105 (2011) 044.
 [10] G. Cullen et al., Eur. Phys. J. C 72, 1889 (2012).
 [11] S. Agrawal, T. Hahn and E. Mirabella, arXiv:1112.0124 [hepph].
 [12] F. Cascioli, P. Maierhofer and S. Pozzorini, Phys. Rev. Lett. 108, 111601 (2012).
 [13] S. Badger, B. Biedermann, P. Uwer and V. Yundin, arXiv:1209.0100 [hepph].
 [14] P. Mastrolia and G. Ossola, JHEP 1111, 014 (2011).
 [15] S. Badger, H. Frellesvig and Y. Zhang, JHEP 1204 (2012) 055.
 [16] Y. Zhang, JHEP 1209 (2012) 042.
 [17] P. Mastrolia, E. Mirabella, G. Ossola and T. Peraro, arXiv:1205.7087 [hepph].
 [18] R. H. P. Kleiss, I. Malamos, C. G. Papadopoulos and R. Verheyen, arXiv:1206.4180 [hepph].
 [19] S. Badger, H. Frellesvig and Y. Zhang, JHEP 1208 (2012) 065.
 [20] B. Feng and R. Huang, arXiv:1209.3747 [hepph].
 [21] J. Gluza, K. Kajda and D. A. Kosower, Phys. Rev. D 83 (2011) 045012.
 [22] D. A. Kosower and K. J. Larsen, Phys. Rev. D 85, (2012) 045017.
 [23] K. J. Larsen, arXiv:1205.0297 [hepth].
 [24] S. CaronHuot and K. J. Larsen, arXiv:1205.0801 [hepph].
 [25] J. Alcaraz Maestre et al., arXiv:1203.6803 [hepph].
 [26] F. Tramontano, in these proceedings.

[27]
R. K. Ellis, W. T. Giele and Z. Kunszt,
JHEP 0803 (2008) 003.
R. K. Ellis, W. T. Giele, Z. Kunszt and K. Melnikov, Nucl. Phys. B 822 (2009) 270;
W. T. Giele, Z. Kunszt and K. Melnikov, JHEP 0804 (2008) 049.  [28] P. Mastrolia, G. Ossola, T. Reiter and F. Tramontano, JHEP 1008 (2010) 080.
 [29] T. Binoth et al., Comput. Phys. Commun. 180 (2009) 2317.
 [30] G. Heinrich, G. Ossola, T. Reiter and F. Tramontano, JHEP 1010 (2010) 105.

[31]
G. ’t Hooft and M.J.G. Veltman,
Nucl. Phys. B 153 (1979) 365;
G. Passarino and M.J.G. Veltman, Nucl. Phys. B 160 (1979) 151;
G. J. van Oldenborgh, Comput. Phys. Commun. 66 (1991) 1;
R. K. Ellis and G. Zanderighi, JHEP 0802 (2008) 002;
A. van Hameren, Comput. Phys. Commun. 182, 2427 (2011);
G. Cullen et al., Comput. Phys. Commun. 182 (2011) 2276.  [32] N. Greiner, A. Guffanti, T. Reiter and J. Reuter, Phys. Rev. Lett. 107, (2011) 102002.
 [33] N. Greiner et al., Phys. Lett. B 713 (2012) 277.
 [34] P. Mastrolia, E. Mirabella and T. Peraro, JHEP 1206 (2012) 095.
 [35] D. Forde, Phys. Rev. D 75 (2007) 125019.
 [36] S. D. Badger, JHEP 0901 (2009) 049.
 [37] G. Ossola, C. G. Papadopoulos and R. Pittau, JHEP 0803 (2008) 042.
 [38] P. Mastrolia, G. Ossola, C. G. Papadopoulos and R. Pittau, JHEP 0806 (2008) 030.
 [39] P. Mastrolia, E. Mirabella, G. Ossola and T. Peraro, arXiv:1209.4319 [hepph].