A nice two-loop next-to-next-to-MHV amplitude in N\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ \mathcal{N} $$\end{document} = 4 super-Yang-Mills

We study a scalar component of the 8-point next-to-next-to-maximally-helicity-violating (N2MHV) amplitude at two-loop level in N\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ \mathcal{N} $$\end{document} = 4 super-Yang-Mills theory; it has a leading singularity proportional to the inverse of the four-mass-box square root and receives contributions from only two types of non-trivial integrals with one-loop infrared (IR) divergences. We compute such two-loop 8-point integrals by taking (double-)collinear limits of certain finite, dual-conformal-invariant integrals, and they nicely give the IR-safe ratio function after subtracting divergences. As the first genuine two-loop N2MHV amplitude computed explicitly, we find remarkable structures in its symbol and alphabet: similar to the next-to-MHV (NMHV) case, there are still 9 algebraic letters associated with the square root, and the latter also becomes a letter for the first time; unlike the NMHV case, such algebraic letters appear at either one or all of the second, third and last entry, and the part with three odd letters is particularly simple.


Introduction
Scattering amplitudes are central objects in fundamental physics: they are crucial for connecting theory to experiments in particle accelerators such as Large Hadron Collider, and they play a central role in discovering new structures of Quantum Field Theory (QFT). In particular, tremendous progress has been made for planar N = 4 supersymmetric Yang-Mills theory (SYM); not only have hidden mathematical structures for all-loop integrands been unraveled [1][2][3], but amplitudes have also been determined to impressively high loops, for n = 6, 7 [4][5][6][7][8][9][10][11][12][13][14] and beyond [15][16][17][18]. A remarkable duality between Maximally Helicity Violating (MHV) scattering amplitudes and null polygonal Wilson loops (WL) of the theory was discovered at both strong [19][20][21] and weak coupling [22][23][24][25][26][27]; later it was established that super-amplitudes (after stripping off MHV tree prefactor) are dual to supersymmetric WL [28,29], and quite a lot of what we have learned about amplitudes are from this duality picture. For example, one can compute amplitudes at any value of the coupling around collinear limits [30] based on integrability [31] and operator product expansions (OPE) of WL [32]. From such a dual WL picture, one can derive the powerfulQ anomaly equation [33], which has been a driving force for computing multi-loop amplitudes, including two-loop MHV to all multiplicities [16], n ≤ 9 Next-to-Maximallly Helicity Violating (NMHV) [17,18,33] and even three-loop MHV for n ≤ 8 [34]. However, this method breaks down for amplitudes with more complicated helicity distribution, i.e. N k MHV amplitudes for k ≥ 2, where k + 2 is the number of external particles with negative helicity.
As shown in [33], given lower-loop amplitudes with higher n, k, theQ anomaly equation can be used to uniquely determine MHV and NMHV amplitudes, up to "constants" which are in the kernel ofQ operator: any function that satisfiesQF n,k = 0 must be a constant JHEP12(2022)158 for k = 0 or constant times R-invariants for k = 1 [33]. However, this is no longer true for k ≥ 2: there exist transcendental functions in the kernel ofQ for N 2 MHV amplitudes and beyond. In principle such amplitudes can be determined by exploiting anomaly equations for level-one generators such as Q (1) , which can be obtained from spacetime parity-conjugation of theQ equation, but it is a formidable task already for the simplest case with n = 8, k = 2. It remains an important open question to determine, or constrain as much as possible, multi-loop amplitudes with k ≥ 2 usingQ and Q (1) anomaly equations; in particular, an important open question which we will not attempt to answer here is what can such equations say about amplitudes which evaluate to functions beyond multiple polylogarithms (MPL) such as n = 10, k = 3 case [35][36][37]?
In this paper, we will take the more traditional approach, namely directly computing Feynman loop integrals contributing to (certain components of) amplitudes with k ≥ 2, which has proved very successful for e.g. two-loop MHV and NMHV amplitudes. The main motivation here is to obtain more data about scattering amplitudes and Feynman integrals in N = 4 SYM, which in turn allows us to discover more underlying mathematical structures and physics related to theQ anomaly equation etc. We are interested in twoloop N 2 MHV amplitudes, where the integrands in four-dimensional space are known from generalized unitarity [38]; at least for n = 8, all such integrals are expected to evaluate to MPLs, which can in principle be done by using direct integration method if infrared divergences are suitably regulated. We will not compute the entire two-loop 8-point N 2 MHV super-amplitude mainly because: (1) there are too many integrals with rather complicated kinematic dependence with as many as 9 dual-conformal-invariant cross-ratios; additional technical difficulties are caused by regulating divergent integrals; (2) we expect that most components of N 2 MHV amplitudes are similar to those of NMHV/MHV amplitudes, since they receive contributions from same types of integrals which results in similarities regarding their symbology; we will focus on what we consider as "genuinely new" components of N 2 MHV amplitudes, which exhibit new structures invisible at NMHV/MHV level.
Therefore, we will focus on a class of particularly nice components of N 2 MHV amplitudes, which vanish at tree level and remain finite at one-loop level. The algebraic (Grassmannvalued) coefficients of these integrals, which are leading singularities or Yangian invariants [2,39], are well understood: for k = 2 only one special class of them are non-rational functions with square roots, which first appear in one-loop amplitudes as coefficients of four-mass box integrals. Certain scalar components isolate such a non-rational Yangian invariant [2,40], thus e.g. at one loop it is simply given by a finite four-mass box integral which contains the same square root. For n = 8, there are exactly two such scalar components related to each other by a cyclic rotation; one of them reads A(ϕ 12 , ϕ 12 , ϕ 13 , ϕ 13 , ϕ 34 , ϕ 34 , ϕ 24 , ϕ 24 ) , which depends on the square root ∆ 1,3,5,7 . It is given by the four-mass box integral with dual points x 1 , x 3 , x 5 , x 7 , which will be denoted as ∆ when there is no ambiguity. At two-loop level, as we will see shortly, such a component receives contributions from three integrals (up to cyclic rotations): a penta-box and a double-box, both of which has only one-loop divergence, and the well-known finite box ladder integral [41]. The finite ratio function JHEP12(2022)158 can be obtained by subtracting one-loop MHV amplitudes multiplied by the one-loop component, which is given by the four-mass box function.
We will use the dual conformal invariant (DCI) regularization [42] since these integrands are defined strictly in four-dimensional space: it turns out the n = 8 penta-box and doublebox can be obtained from double-collinear limits of n = 10 finite DCI integrals, and the DCI regularization allows us to extract these divergent integrals from the latter: by sending a dual point to infinity for the n = 10 penta-box integral, it is nicely reduced to some two-loop master integrals with four masses which have been computed very recently using differential equations [43]; the n = 10 double-box evaluates to elliptic multiple polylogarithms [37], but we will see that it suffices to take a double-collinear limit for its one-dimensional integral representation, which gives (MPL) n = 8 double-box. After subtracting the DCIregulated one-loop 8-point MHV amplitude multiplied by the four-mass box, we confirm the cancellation of divergences and end up with a finite ratio function.
Having computed these cutting-edge examples for two-loop DCI-regulated integrals contributing to this N 2 MHV component, we will then study the structures of the resulting symbol and its alphabet, especially in comparison with earlier results of n = 8 NMHV and MHV amplitudes [16,17,34]. Recall that the NMHV alphabet consists of 180 rational letters and 9 + 9 algebraic letters associated with square root ∆ and its cyclic rotation(MHV case is absent of any square root) [17], and the appearance of these algebraic letters has been studied from many different directions [44][45][46][47][48][49][50][51][52][53][54][55][56]). Here we find that the alphabet of this component (and its cyclic rotation) stays very similar to the NMHV case; in particular there are still 9 independent algebraic letters which are odd under the flip ∆ → −∆ (all rational letters are even), and there is exactly one new letter for this N 2 MHV component, namely ∆ itself. Furthermore, recall that NMHV amplitudes or other components of N 2 MHV amplitudes must be even under the flip, thus at two loops they contain none or two odd (algebraic) letters, which can only be in the second and third entry [17,18] (some individual Feynman integrals also have this property [57,58]). In particular this means that the last entry only consists of even (rational) letters, as predicted byQ equation. On the contrary, this special component of N 2 MHV must be odd for the flip, and at two loops it contains either one or three odd letters, which can appear in the second, third and last entries. We will find remarkably simple results for the part containing three odd letters.

A nice component of 8-point N MHV: two-loop ratio function
A nice representation for two-loop integrands of n-point, N k MHV super-amplitude in N = 4 SYM has been obtained using generalized unitarity [38]. Schematically, the amplitudes in planar N = 4 SYM take the form where leading singularities are Yangian invariants: they are completely fixed by super conformal symmetries and dual super conformal symmetries and hence independent of loop level [2].

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For our purpose, it is convenient to work with the dual superspace coordinates (x, θ), as well as the following shorthand notation for the Lorentz invariants, To linearly realize the dual superconformal symmetries and have nice expressions for Yangian invariants, it is convenient to introduce (super) momentum twistor variables [59], In terms of super momentum twistors, we further define the basic SL(4)-invariant ijkl := or the Plücker coordinates of Gr(4, n)), and the basic R invariant [60,61] The genuine N 2 MHV amplitudes in planar N = 4 SYM first appear starting from n = 8, which is sufficient for our purpose. As we have mentioned, we are mostly interested in (two cyclically related) component amplitudes, which are proportional to Yangian invariants with square roots; such a scalar component reads: 8,2 receives contribution only from one term in eq. (2.1), where α and δ are two solutions of the Schubert problem and By integrating Grassmannian variables, we have the scalar component A JHEP12(2022)158 x 5 x 8 x 0 x 8 x 0 x 6 x 5 x 0 x 7 x 0 Figure 1. Three Feynman diagrams as well as their dual diagrams that contribute to the two-loop N 2 MHV component amplitude A 8,2 : the penta-box diagram, the double-box diagram, and the boxladder diagram. In the dual diagrams, the line connecting to two dual points, x a and x b , represents a factor x 2 a,b in the denominator, while the dotted line represents a factor in the numerator.
where the box integral has been denoted as the one-loop instance of well-known box ladders [41], I bl , and z,z, 1 − z, 1 −z, which contains the square root ∆, are defined by At two-loop level, by repeating the procedure as in the one-loop case, one can find only three types of Feynman integrals that contribute to this component amplitude: up to cyclic rotations, we have a penta-box integral with 5 dual points, I pb (x 1 , x 3 , x 5 , x 7 , x 8 ), a double-box integral with 6 dual points, I db (x 1 , x 3 , x 5 , x 6 , x 7 , x 8 ), and the double box integral with 4 dual points I (2) bl (x 1 , x 3 , x 5 , x 7 ) (L = 2 instance of the box ladder I (L) bl ) [41]: (2.10) where these three types of Feynman integrals read the factor '2' in front of I pb and I db is due to their symmetry under the exchange x 0 ↔ x 0 , '+3 cyclic' means taking x i → x i+2 for i = 1, . . . , 8 which gives a cyclic orbit of length 4.
As remarked in the introduction and shown in the one-loop case eq. (2.9), this component amplitude A 8,2 as well as its three ingredient integrals are pure polylogarithms divided by JHEP12(2022)158 the square root we thus introduce the normalized amplitudes and Feynman integrals indicated by a hat: (2.14) This component suffers from infrared divergence: both the penta-box integral I pb and double-box integral I db has one-loop divergence from the box with two massless legs (x 0 in the above equations). However, it is well known that the infrared divergence is captured by the MHV amplitudes (also known as BDS ansatz) [62], then it is clear that the so-called ratio functions R n,k = A n,k /A n,0 are finite and independent of the regularization scheme. For our case, the corresponding component of R 8,2 is slightly simpler and reads due to the vanishing A (0) 8,2 . As above, we introduce the normalized (pure) ratio function R 8,2 . The infrared structure of A (2) 8,2 now is manifest: it is captured by the one-loop 8-point MHV amplitude A 8,0 . Note that this component ratio function is the same as the BDS-normalized amplitude The general regularization for the Feynman integrals in Gauge theories is dimensional regularization which will spoil the dual conformal symmetries of N = 4 SYM, we instead use the so-called dual-conformal regularization [42], which will be elaborated in the following section.

The computation: DCI-regulated penta-box and double-box integrals and the subtraction
The infrared divergences of the penta-box integral and the double-box integral arise from massless legs of the box sub-integral (on the right, see figure 1): for the penta-box, x 2 7,8 and x 2 8,1 vanish, and so do x 2 6,7 and x 2 7,8 for the double-box. To regulate these divergences, the most straightforward way is to assign a small mass µ to these massless legs, then take the limit µ → 0, which is also known as the Higgs regularization [63,64]. In the dual space, this corresponds to shifting dual points by the dimensional parameter µ which breaks the dual conformal symmetries. The dual conformal regularization [42,65] instead shifts each dual point (for a = 1, 2, . . . , n) by

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where the finite weight-2 functions read with dual conformal cross-ratios Similarly, one can compute one-loop n-point N k MHV amplitudes A n,k with this regularization, and obtain the finite ratio function at one-loop level: R n,0 , where log 2 and log terms cancel nicely [42].
Moving to our two loop computation, in eq. (2.15) we also need to regulate the pentabox integral and the double-box integral with one-loop divergences besides A 8,0 . Their results in dual conformal regularization can be obtained as special double-collinear limits of their finite counterparts with n = 10, which are already known from the literature [37,43]. In the rest of this section, we will elaborate the procedure of taking such collinear limits. x 3 x 1 x 10 x 8 which is finite and depends on 7 cross-ratios . (3.6) One can easily see that this integral reduces to x 2 1,5 x 2 3,7 I db in the collinear limit x 10 → x 8 , x 8 → x 7 at the integrand level. The elliptic double-box integral has been evaluated as elliptic multiple polylogarithms in [37], where its symbol is also given. However, a better start point turns out to be its one-fold integral representation given in [37] where G 3 (x, y) is a known MPL of weight 3, which depends on 7 cross-rations, as well as {x, y} given by the elliptic curve

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with (3.9) Now let us turn to the 8-point double box. With the DCI regulator eq. (3.1), the 7 cross-ratios in eq. (3.6) behave like as → 0. Correspondingly, the elliptic curve eq. (3.8) degenerates to and G 3 (x, y) in eq. (3.7) simplifies dramatically as where G fin 2,3 are MPLs of weight 2 and 3, respectively. A nice observation is that for the log 2 term, the integral log (1+x)(x+u) xv dx (x+z)(x+z) indeed evaluates to the four-mass box integral 1 ∆ A 8,2 in eq. (2.9). This already provides some preliminary evidence that IR divergences will be cancelled in (2.15) to give a finite result. It is straightforward to evaluate the remaining integrals G fin 2,3 dx (x+z)(x+z) with, say HyperInt or PolyLogTools [66,67]. Here we only record the symbol [68] of its cyclic image I db (x 5 , x 7 , x 1 , x 2 , x 3 , x 4 ), which can be obtained much easier by the algorithm provided in appendix A of [33] (which is also reviewed in appendix A of this paper), in the supplementary material attached to this paper n82Lnnmhv_scale_component.txt as variables puredb$log2e, puredb$loge and puredb$finite.
The penta-box integral. The 8-point penta-box integral I pb can be obtained as a double-collinear limit of the 10-point penta-box integral, which we can compute in principle in Feynman-parameterized form, but the computation turns out to be rather tedious. Fortunately, we find that the 10-point penta-box integral belongs to the family of integrals recently computed in [43] by canonical differential equations: the penta-box integral can be identified as a non-DCI double box integral by sending x 5 to ∞, see figure 2. This non-DCI limit gives us a bijection between the kinematics of these two Feynman integrals, (3.13) For external Mandelstam variables, namely x 2 i,j with i, j = 0, 0 , we can further write them in terms of momentum-twistor variables 14)

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x 7 x 8 where the infinite bi-twistor I ∞ is identified as the line (45) since we have taken x 5 → ∞.
The non-DCI double-box integral I nDCI-db is denoted in [43] as G 1,1,1,1,1,1,1,−1 , which can be expressed as linear combination of the following three master integrals I 5 = r 9 G 0,1,1,1,1,1,1,0 , I 6 = r 8 G 1,1,0,1,1,1,1,0 where we have used (see the figure 2 above for definition of D i 's): Therefore, I nDCI-db = G 1,1,1,1,1,1,1,−1 can be solved as where I 3 , I 5 and I 6 are three pure weight-4 MPLs, and r 2 , r 8 , r 9 are three different square roots of kinematics variables given by Applying the bijection eq. (3.13) and then taking double-collinear limits with DCI regulator leads to we then get the full result of the 8-point penta-box integral I pb in the DCI regularization. Under the collinear limits eq. (3.16), only the square root r 2 survives: 17) and this implies that the divergent penta-box integral shares the same overall factor, the square root (x 2 1,5 x 2 3,7 ∆) −1 , with the divergent double-box integral. Since the coefficients of JHEP12(2022)158 I 5 and I 6 in eq. (3.15) vanish, we here only need to consider the collinear limit of I 3 . By taking the collinear limit of its letters and keeping the leading terms of in the symbol, we find that I pb has the expected IR divergence structure and takes the form pb are two finite, pure MPL functions of weight 3 and 4 respectively. In the supplementary material attached to this paper n82Lnnmhv_scale_component.txt, the three terms of S ( I pb (x 3 , x 5 , x 7 , x 1 , x 2 )) are stored in three variables purepb$log2e, purepb$loge and purepb$finite.
The subtraction. Now we move to the subtraction in (2.15) which should give an IR finite ratio function. The cancellation of leading divergences, i.e. the log 2 ( ) part, is easy to see. Since the log 2 ( ) divergence of both penta-box and double-box integrals is given by the pure function A (1) 8,2 , by summing over their cyclic images (see eq. (3.2)) in the ratio function, we see that log 2 ( ) divergence is cancelled perfectly.
What is much more non-trivial, is the cancellation of sub-leading log( ) divergences in the ratio function. Note that the log( ) part of both double-box and penta-box integrals is given by complicated weight-3 MPL functions, which certainly look much more complicated than the subtraction term in (2.15). We find it totally remarkable that in the cyclic sum, all these complicated weight-3 MPL functions combine into precisely the log( ) part of the eq. (3.2), namely simple logarithmic functions times A (1) 8,2 . This provides a very nontrivial consistency check of our computations for both DCI-regulated integrals, and such a precise cancellation of all IR divergences produces a finite result for the ratio function. We record its symbol in scalecomponent in the supplementary material attached to this paper n82Lnnmhv_scale_component.txt, and we also provide its alphabet as the variable alphabet for convenience.

The symbol and alphabet of the ratio function
In this section, we discuss the symbol and alphabet of the ratio function, R 8,2 . The full symbol is too lengthy to be present here, and we record it in a file in the supplementary material attached to this paper. Here we briefly comment on certain structures we find in the symbol of R (2) 8,2 , especially some new features compared with NMHV and MHV cases. A new feature of this component of N 2 MHV amplitudes, as opposed to other components of NMHV/MHV amplitudes, is that the symbol is odd with respect to the flip ∆ → −∆. This is due to the fact that its leading singularity is proportional to (the inverse of) ∆. Thus, similar to the one-loop component (four-mass box function) but for the first time for two-loop amplitudes, each term of the symbol (a "word") contains odd number of odd letters, which are algebraic (non-rational) functions of momentum twistors. Recall that for one-loop case, the symbol reads

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which is odd under ∆ → −∆ since it contains odd letters z/z, (1 − z)/(1 −z) in the second entry, e.g. log(z/z) → − log(z/z) under the flip. Similarly at two-loop level, since the first entry must be even letters, there is either one such odd letter at the second, third and fourth entry, or all these three entries are odd. In particular, this is the first example of N = 4 SYM amplitudes at two-loop level where the last entry can be odd letters. Recall that for the two-loop 8-point NMHV amplitude we find 9 multiplicatively independent algebraic letters that are odd in ∆ → −∆) associated with this square root (and 9 more related by a cyclic rotation i → i+1). It is nice that this component of the two-loop 8-point N 2 MHV amplitude still contains exactly this 9-dimensional space of odd letters, and we denote them as {χ(a 1 ), χ(a 2 )}| i→i+2k for k = 0, 1, 2, 3 and Our result strongly supports the conjecture that altogether the 9 + 9 letters constitute all algebraic (odd) letters for n = 8 amplitudes for all helicity sectors.
Next we move to even letters, which are rational functions of momentum twistors. We note that again almost all of them (together with those for the other component, related by i → i+1) have been seen in the alphabet of n = 8 NMHV amplitudes: they are 92 polynomials of Plücker coordinates, which can form 92 − 8 = 84 DCI combinations. There are 56 Plücker coordinates (4-brackets): under cyclic rotations i → i+2 they form 13 length-4 orbits and 2 length-2 ones, with 15 seeds chosen as   1234 , 1235 , 1236 , 1237 , 1238 , 1245 , 1248 , 1256 , 1258 , 1267 , 1268  In addition to these letters which have appeared in NMHV/MHV amplitudes, we find exactly one new letter, which is nothing but the inverse of leading singularity, ∆! Let us briefly comment on how the letters appear in the symbol. As indicated by physical discontinuity conditions [69], we find exactly 20 letters of the form i i+1 j j+1 JHEP12(2022)158 which appear in the first entry; the frozen ones i i+1 i+2 i+3 (for i = 1, . . . , 8, treated as 2 length-4 orbits above), and 3 length-4 orbits generated by seeds 1245 , 1256 and 1267 . The first two entries respect Steinmann relations, and we find that all first two entries are consistent with the general prediction of [70]: they are either log log terms respecting Steinmann relations, or the symbol of one-loop box functions i.e. I (1) (x 1 , x 3 , x 5 , x 7 ) and finite part of its lower-mass degenerations and a length-2 orbit { 1458 , 2367 }.
In particular, those terms with 3 odd letters are very simple: the first-two entries can only be the symbol of the four-mass box, eq. (4.1), and we record the last-two (odd) entries: in principle we have 9 × 9 terms but the result is much more compact, which we record as Alternatively, if we denote χ i := v i and χ i := v i+4 for i = 1, . . . , 4 and χ := v 9 , we can write this symmetric, weight-2 word as the symbol of where the remaining terms have one odd letter in either second, third or last entry. These terms involving only one odd letter seem to be significantly more complicated. For example, for terms where only the second entry is odd (χ(0) or χ(1)), the first two entries must again form the symbol of I (1) bl , while the last two entries consist of even letters, including the new letter ∆.

Conclusion and outlook
In this paper, we have computed a particularly nice component of the two-loop 8-point N 2 MHV amplitude, whose leading singularity is proportional to the inverse of the four-mass square root, which makes it distinct from other N 2 MHV components. The component receives contributions from only two new integrals, which we have computed using the DCI regularization and the finite ratio function is obtained by subtracting IR divergences. This is the first two-loop amplitudes beyond MHV and NMHV cases that have been computed, and the resulting symbol has several interesting features; compared to NMHV case it contains exactly one new letter, which is the square root itself, and either one or all of the last three entries must be algebraic (odd) letters. We have found a remarkable simplicity for the latter case, see (4.8) and (4.9).
There are several directions worth further investigations. Two immediate generalizations are (1) computing all components of the two-loop 8-point N 2 MHV amplitude, which should be straightforward but rather tedious; (2) computing such special components for n-point N 2 MHV amplitudes, e.g. 9 such components each with a square root for n = 9 case. Our techniques should be applicable but several new cases of penta-box integrals etc. are needed. It would be interesting to look for more structures in the symbol and alphabet of such special components for n = 8 and higher, similar to what we have considered for NMHV and MHV cases, and it would also be nice to further study mathematical structures in the symbol of such two-loop integrals (see [53,54,56,70,71] and references therein). Another important open question is how to uplift these symbols to functions or directly bootstrap them. Now that we have some control of n = 8 MHV, NMHV and components of N 2 MHV amplitudes, we could compare them in more details.
It would be highly desirable to study what do such structures, especially the appearance of algebraic letters in the last entries, mean for theQ and Q (1) anomaly equations, and eventually use them to compute amplitudes with k ≥ 2. In this regard, we can try applying these anomaly equations for certain components rather than for the complete super-amplitude (related anomaly equations have been applied to other theories and even individual integrals in [72,73]). Last but not least, we have further demonstrated how DCI-regulated integrals are useful for computing IR-safe quantities for loop amplitudes with higher multiplicities. It would be interesting to push this direction further, including the computation of non-planar SYM amplitudes and those in supergravity theories [74,75], as well as amplitudes in other theories (such as ABJM, see [76,77]).
The entries of a symbol are called its letters, and the collection of all letters is called its alphabet. For our calculation, it's more convenient to perform integrations on the symbol level directly based on the following rules [33]: suppose we have an integral b a d log(t + c) (F (t) ⊗ w(t)), where F (t) ⊗ w(t) is a linear reducible symbol in t, i.e. its entries are products of powers of linear polynomials in t, and w(t) is the last entry. The total differential of this integral is the sum of the following two parts: (1) the contribution from endpoints:
The algebraic letters are the same for the 3-loop MHV octagon and the two-loop NMHV octagon, which are cyclic images of eq. (4.2) by taking i → i + 1.
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