N 3 LO gravitational quadratic-in-spin interactions at G 4

,


Introduction
As of 2016 the observation of gravitational waves (GWs) has become a reality [1].An unexpected variety of GW events has already been observed from black hole and neutron star binary mergers on the first and second observation runs of the LIGO and Virgo collaborations [2][3][4].The continuously increasing influx of data expected from the expanding worldwide network of ground-based interferometers [5][6][7][8] and anticipated space-based detectors in complementary frequencies [9,10] places significant demands on the precision of theoretical predictions.The theoretical waveform templates used for these observations are uniquely created using the effective one-body (EOB) framework [11,12], which in turn relies heavily on the post-Newtonian (PN) theory of General Relativity as input [13].Even relatively high-order corrections beyond Newtonian gravity, such as the sixth PN (6PN) order, are required for accurate waveforms, and to gain further information about the inner structure of the individual components of the binary.
PN theory provides an analytic treatment of the long inspiral phase, in which the two compact objects in the binary move with non-relativistic velocities.The orbital dynamics of the compact binaries is an essential ingredient for theoretical waveform models.The current state of the art for orbital dynamics for generic compact binaries in PN theory is presented in table 1.This table shows the sectors obtained at order n + l + Parity(l)/2 in the PN expansion, where l is the order of spin that appears in the sector with the corresponding parity for even or odd l, and for l ≥ 2 finite-size effects have to be tackled.Along the years much of the progress in PN theory has been made only for the simple unrealistic case, in which the compact objects are not spinning and are considered as point-masses (corresponding to the first row in table 1), due to the considerable conceptual and computational difficulty of treating spinning objects in gravity.
Nevertheless, in recent years remarkable progress has also been made in the spinning sectors via the effective field theory (EFT) approach to PN gravity [14,15] within the ❍ ❍ ❍ ❍ ❍ ❍ l n (N 0 )LO N (1) LO N 4 24 S 4  3 5 Table 1.The minimum number of n-loop graphs within the EFT framework for each PN sector that has been completed to date for the orbital dynamics of generic compact binaries.The gray area indicates the sectors that correspond to gravitational Compton scattering with quantum spins framework of the EFT of gravitating spinning objects [16].The filled entries in table 1 show the number of n-loop graphs that contribute within the EFT framework in each N n LO sector that has been completed to date.The boldface entries in the table have been completed only via the EFT of gravitating spinning objects [16], in a series of works [17][18][19][20][21][22][23][24][25][26].In particular, in [16] the leading non-minimal gravitational couplings to all orders in spin were formulated, thus enabling the completion of all sectors with finite-size effects up to the current state of the art at the 4PN order.
This line of work was recently extended along both of the axes of table 1: The first three-loop calculation in the spinning sector was computed in [25], using the publiclyavailable EFTofPNG code [23], and the cubic-and quartic-in-spin sectors were tackled at one-loop level in [24,26].The latter sectors thus uniquely explore the gray area in table 1, which corresponds to gravitational Compton scattering with quantum spins s ≥ 3/2, as sectors with classical spin at the l-th order correspond to scattering with quantum spin of s = l/2 [27].Altogether, this has been pushing the precision frontier to the 5PN order.This work derives for the first time the complete N 3 LO gravitational interactions which are quadratic in the spins from a diagrammatic expansion at order G 4 .All contributions at this order are static, meaning that they involve no explicit factors of the velocities of the compact objects.This sector involves both three-loop graphs and finite-size effects due to the spin-induced quadrupole.It enters at the 5PN order for maximally-spinning compact objects, thus further pushing the precision frontier of PN gravity.This work builds on the EFT of gravitating spinning objects [16] and its implementation in the publicly-available EFTofPNG code in [23], as well as on their recent implementations and upgrade at the two-loop level [21] and at the three-loop level [25].
As noted above the spinning sectors are considerably more challenging to handle than the non-spinning ones.First, contrary to the non-spinning case, in the spinning sectors all possible graph topologies are realized at each order of G [28].While there are no threeloop graphs that enter in the non-spinning N 3 LO sector, in the present sector there are 52 such graphs (see table 1), which turn out to be precisely those that produce divergences and logarithms.Further, this sector contains 163 graphs to evaluate compared to only 8 in the N 3 LO sector without spins.We also recall that spins are derivatively coupled, which in this sector with two spins leads to integrand tensor numerators up to rank eight, comparable to N 5 LO in the sector without spins.Finally, at this order we also have to consider further contributions from higher-order operators with spins that are beyond linear in the curvature (note, however, that tails that involve spin couplings do not contribute at the order considered here [13,29]).
The paper is organized as follows.We begin in section 2 by reviewing the formal framework of the EFT of gravitating spinning objects, which we extend in section 2.1 to include further non-minimal couplings in the effective action of a spinning particle that become relevant at this order.We proceed in section 3 to consider the diagrammatic expansion of interactions that are quadratic in the spins, highlighting how the graphs in this sector can be constructed out of the graphs in lower-order sectors.We discuss the total outcome for the sector in section 4, and conclude in section 5.

EFT of gravitating spinning objects
We start by reviewing the framework of the EFT of gravitating spinning objects, which enables our derivation of the N 3 LO quadratic-in-spin sectors from a diagrammatic expansion at order G 4 .We follow closely the setup presented in the recent work [25] and also build on [21], keeping similar conventions and notations.First we will extend the one-particle effective action that was required for the N 3 LO spin-orbit in [25], introducing further Feynman rules that are required in this sector.Thus, from the two-particle effective action that describes a compact binary [14,15]: we will only be concerned with S pp , the worldline action of a spinning particle for each of the two components of the binary, where λ a are their respective worldline parameters.
From the pure gravitational action, S g , given in [25] in the harmonic gauge, no additional ingredients are required beyond those presented in [25].Hence, we use similar propagators for the gravitational field components in terms of the Kaluza-Klein (KK) decomposition [30,31], and no further bulk vertices are required beyond those which were added in [25].As in [25] the spatial dimension, d, is kept generic throughout, which also matches what is done in the EFTofPNG code [23].We use the corresponding d-dimensional gravitational constant [25], where G N ≡ G is Newton's gravitational constant in three-dimensional space, γ is Euler's constant, and R 0 is a fixed renormalization scale.This corresponds to the modified minimal subtraction (MS) prescription in dimensional regularization used in this work, see e.g.[32].As in the N 3 LO sector at order G 4 in [25] relativistic corrections to the propagators are not relevant in this paper.
We now focus on the point-particle action for each of the spinning particles [15,16].The quadratic-in-spin sector includes three types of interaction: i. the coupling between the spins of both objects, referred to as the spin 1 -spin 2 interaction, ii. the nonlinear interaction of each object's spin with itself, referred to as spin 1 -spin 1 interaction, and iii.finite-size effects that involve the spin-induced quadrupole of each of the rotating objects.Due to the latter interaction, the effective action should be considered beyond minimal coupling, which is sufficient for the spin-orbit sector, and for interactions that are dependent on the linear spin couplings as in the spin 1 -spin 2 and spin 1 -spin 1 interactions.Considering all these interactions, the effective action of each of the spinning particles reads [15,16]: where L N M C denotes the non-minimal coupling part of the action induced by the spin of the object.This part is initially formulated in terms of the definite-parity pseudovector S µ , as defined in [16,19,24].Beyond these non-minimal couplings all of the previous terms in the action are similar to what is noted in [25], where the difference with the action in [33][34][35] was highlighted.
The non-minimal coupling part of the effective action involving the spin was constructed in [16], where the spin-induced non-minimal couplings to all orders in spin and linear in the curvature were derived to be: which involves new spin-induced Wilson coefficients, the electric and magnetic curvature components of definite parity, defined as as well as their covariant derivatives, D µ .Of the infinite series in eq. ( 2.4) only the first operator is required in this paper, corresponding to the spin-induced quadrupole that reads: Up to missing generic symmetry and construction considerations, a closely related expression was used in [36], which conformed with the well-known LO spin-squared interaction from [37,38].
There are no additional Feynman rules (such as worldline mass and spin couplings) required for the spin 1 -spin 2 and spin 1 -spin 1 interactions, which originate from the minimalcoupling part of the point-particle action, beyond those presented in [20,25].Thus, we turn now to the Feynman rules required for this sector due to the interaction involving the spin-induced quadrupole, which go beyond the rules in previously computed lower-order spinning sectors [21].All of the aforementioned Feynman rules can be obtained within the public EFTofPNG code [23] for a generic number of spatial dimensions d.The new relevant Feynman rules for this sector were obtained by further extending the FeynRul module of the EFTofPNG code [23].
For the three-graviton coupling to the worldline spin-induced quadrupole, the new required Feynman rule is while there is also a new Feynman rule for the four-graviton coupling to the worldline spin-induced quadrupole, given by (2.9) We remind the reader that these rules are already given in terms of the physical spatial components of the local Euclidean spin vector in the canonical gauge [16], and that all of the indices are in fact Euclidean.

Extending the EFT of a spinning particle
To complete the effective action at this order in PN accuracy in the spinning sectors [21,25] including the current sector, we extend the non-minimal coupling part of the effective action of a spinning particle given in eq.(2.4).This extension contains operators that are quadratic in the curvature components and hence stand for tidal deformations of the extended compact object.Following similar symmetry considerations and the logic outlined in [16], we find that the new terms to quadratic order in spin are given by These terms involve new tidal Wilson coefficients (that in contrast with eq.(2.4) are defined here to absorb all numerical and mass factors).
In the first line of eq.(2.10) we have written the leading mass-induced quadrupolar tidal deformations, which are known to enter at the 5PN order [15], and have suppressed higher-order mass-induced tidal operators, which can be found in [39].We have additionally shown the adiabatic tidal operators which involve the spin up to quadratic order.From dimensional analysis and power-counting considerations (as explained in [15,16]), one can infer that the terms in the second line of eq.(2.10) enter at the 5PN order, while the terms on the third and fourth lines of eq.(2.10) enter only at the 6.5PN and 7PN orders, respectively.
Therefore at the 5PN order considered in this work there are two new operators which are quadratic in the spin and quadratic in the curvature.However, the leading contribution from these operators at the 5PN order shows up in the two-graviton exchange topology at order G 2 (see e.g.figure 2(a) in [25]), and is therefore not relevant in the current paper, but rather will be addressed in a subsequent publication.Notice that interestingly if this expansion that is quadratic in the curvature is continued to higher orders in spin as in [26], only spin orders l = 0, 2, 4 that relate to bosons of quantum spin s = 0, 1, 2 enter at leading order.Spin orders that correspond to fermions and quantum spin s > 2 all require additional covariant derivatives and enter at higher orders.

Perturbative expansion of quadratic-in-spin interactions
In this paper we evaluate the contribution to the N 3 LO sector that is quadratic in the spins, and originates from Feynman graphs at order G 4 in the diagrammatic expansion of the two-particle effective action in eq.(2.1).A comprehensive analysis of the generic topologies at order G 4 in the EFT framework was presented in the recent work [25].Using the terminology defined in that work, these topologies are shown in figure 1, classified according to their self-interaction vertices and the corresponding loop order in the worldline picture [25].As in [25], it is only the graphs that are at three-loop order in the worldline picture that genuinely represent a higher level of complexity in the N 3 LO spinning sectors.These graphs have topologies (d), (f), or (g), as depicted in figure 1 (see also figure 12 in [15]).
As of the two-loop order we also have higher-rank topologies, which means that more than a single basic integral of n-loop form, as specified in [25], is required to express integrals of that topology.In general, a rank-r topology requires a combination of r of the basic n-loop integrals (at order G n+1 ).In this sector at order G 4 we have four higher-rank topologies: Topology (e8) is a rank-two topology, whereas topologies (f5), (g4), and (g5), are rank-three topologies [25].In contrast to the rank-one topologies, which easily boil down to one-loop computations, the higher-rank topologies require considerable processing mainly by means of integration-by-parts (IBP) [40].
We proceed to the construction of the Feynman graphs that contribute to this sector.We recall that the spinning sector is more complicated than the non-spinning sector, because all possible topologies are realized at each order in G, even when the KK field decomposition is used [28,30,31], in contrast to the non-spinning sector, where in particular at N n LO for odd n, n-loop graphs are absent, as can be seen in table 1.As we noted in section 2 this sector contains three types of interactions of two distinct origins: There are the spin 1 -spin 2 and spin 1 -spin 1 interactions, which originate from the minimal coupling part of the action of a spinning particle in eq. ( 2.3), and the interaction that involves the spin-induced quadrupole, which originates from the non-minimal coupling part of the action.
Graphs with the first two types of interaction are readily constructed as subsets of the corresponding graphs in the N 3 LO spin-orbit sector [25] by replacing in the graphs of the latter some of the worldline mass couplings to the gravito-magnetic vector with its leading linear spin couplings.The presence of two spin couplings among the worldline insertions leads to fewer unique graphs than in the N 3 LO spin-orbit sector, but still more than were present in the non-spinning sector.Graphs with the third type of interaction can similarly be obtained as a subset of the non-spinning N 3 LO sector [41,42] by replacing some of the worldline mass couplings to the scalar graviton with its leading spin-quadrupole coupling, or by adding a scalar graviton exchange to the few graphs at order G 3 that can be made static as a result (we remind the reader that this even-parity sector is static at order G 4 ).
Therefore, as no three-loop graphs enter at this order in the non-spinning case when the KK field decomposition is used, there are in fact no three-loop graphs with the spin-induced quadrupole which contribute to the N 3 LO quadratic-in-spin sector; The only contribution to this sector dependent on the spin-induced quadrupole comes from graphs below threeloop order in the worldline picture, as can be seen in figure 6.Note that this is exactly what happens in the NLO spin-squared sector [16] due to the absence of one-loop graphs at the NLO non-spinning sector with the KK fields [30].Altogether, this reasoning provided a complete crosscheck for the automated generation of the Feynman graphs using the FeynGen module of the EFTofPNG public code [23], which was extended to handle this sector.The resulting graphs are drawn in figures 2-6 below (using JaxoDraw [43,44] based on [45]).
There are in total 163 distinct graphs in this sector.Of these 52 are three-loop graphs with spin 1 -spin 2 and spin 1 -spin 1 interactions, as shown in figures 3 and 5, respectively.There are 31 higher-rank graphs to evaluate.Of these 12 are rank-two and 19 are rankthree.The evaluation of the graphs was carried out using the upgrade to the publicly available EFTofPNG code which was described in [25], where the higher-rank graphs are reduced using projection [46][47][48] and IBP [49] methods.Due to the additional spin with respect to the spin-orbit sector further projection of the numerators of the integrands was required.Further, more integrals show up in this sector compared to the corresponding spin-orbit one.
In the ancillary files to this publication we list the values of each of the Feynman graphs, both in PDF form and in machine-readable form.We recall that all of the graphs in figures 2-6 should be accompanied by their 'mirror' graphs, in which worldline labels are exchanged, namely 1 ↔ 2. We note that for the spin-squared interactions in figures 4-6 we present the value for the graph with the spins on worldline "1", while for the spin 1 -spin 2 interaction in figures 2-3 we present the value for the graph with higher power of m 1 .Two independent implementations of the framework outlined thus far were carried out in the present work in order to crosscheck and verify all the new results we present.
Similar features to those which were noted in [25] are observed in this sector, with the new ones (which did not appear below N 3 LO) similarly originating uniquely from three-loop topologies in the worldline picture.Let us enumerate the notable features encountered: 1. Zeros.There are 15 graphs that vanish, 13 of which have topologies (c1) and (e4): these vanish due to contact interaction terms, as discussed in [25].In addition, the graphs 4(e8.1),4(e8.2) vanish, which was expected since these factorizable graphs contain the vanishing graph in figure 6(c1) in the N 2 LO spin-squared sector [21] as a subgraph.

Divergences and logarithms.
There are 36 graphs, which make up the majority of the three-loop graphs, that give rise to simple poles in the dimensional parameter ǫ ≡ d − 3 in conjunction with logarithms in r/R 0 , where R 0 is some renormalization scale.They appear in virtually all three-loop topologies (except (d2), (f3), (g2)) and are discussed in [25].
We recall that the ζ(2) terms or the poles and accompanying logarithms originate independently from different basic integrals as explained in [25].
4 N 3 LO gravitational quadratic-in-spin action at G 4 Summing all graphs at order G 4 , we obtain the following contribution to the N 3 LO gravitational quadratic-in-spin action : with and where r ≡ r 1 − r 2 and n ≡ r/r.Interestingly, in contrast to the situation in the N 3 LO spin-orbit sector [25], all divergent terms, logarithms, and factors of ζ(2) that appear in the individual graphs leading to eqs.(4.2) and (4.3) conspire to cancel out from the final result, which contains only finite rational terms.This is similar to the situation within analogous EFT derivations in the non-spinning sector, where all the poles in ǫ, logarithms, and Riemann zeta values conspire to cancel out in each of the N n LO sectors at G n+1 as known for n ≤ 5 [50,51].We recall that both the non-spinning sector and the present one are static at the highest order in G, and have even parity with respect to the order of spin (see table 1).This contrasts with the odd-parity spin-orbit sector, where the analogous piece is non-static.It is curious then whether this occurrence carries over to all of the even-parity sectors in spin.
In any case, we know that the appearance and treatment of divergent terms and logarithms is related to the treatment of terms with higher-order time derivatives [13].Since the appearance of higher-order time derivative terms is delayed by one order in the quadratic-in-spin sectors with respect to the spin-orbit sector, where it occurs already at the LO [52], it may have been expected that the related novel features that show up in the final N 3 LO spin-orbit result are absent from the final N 3 LO quadratic-in-spin result here.

Conclusions
In this paper we derived for the first time the complete static N 3 LO gravitational interactions that are quadratic in the spins in inspiralling compact binaries from Feynman diagrams with topologies at order G 4 within the framework of the EFT of spinning gravitating objects [16].The derivation builds on the recent work in [25], in which an upgrade of the EFTofPNG public code [23] was carried out, with further extensions required for the present sector.The contribution we have calculated in this paper constitutes the most computationally challenging piece of the N 3 LO quadratic-in-spin sector in terms of integration, due to the three-loop level that is the highest loop level in this sector.This sector enters at the 5PN order for maximally-spinning compact objects, and complements the non-spinning sector at the same order, with relevant pieces in e.g.[50,51] and [53].
This sector contains three types of interactions that originate from the two distinct parts of the effective action of a spinning particle, where in particular one interaction involves finite-size effects, which arise from the non-minimal coupling part of the pointparticle action.Such effects distinguish between black holes and neutron stars, in contrast to the spin-orbit coupling or point-mass interactions.Further, at this PN order higher nonminimal coupling operators beyond linear in the curvature with spin need to be included for the first time.We have correspondingly extended the effective action formulated in [16] to include operators that are quadratic in the curvature, similar to [26] at the same PN order.While we find such operators that are quadratic in spin, and that can enter at this PN order, they do not enter at this order in G 4 , and are thus left to a forthcoming publication.
The N 3 LO quadratic-in-spin interactions consist of a total of 163 unique graphs at order G 4 .Of these 52 are three-loop graphs, which arise uniquely from the interactions that originate from minimal spin coupling, and in which special features are observed, similar to the analogous sector in the spin-orbit interaction [25].However, these features (including divergences, logarithms, and transcendental factors) conspire to cancel out in the final result, similar to what happens in the non-spinning sector within EFT derivations for n ≤ 5 in the N n LO sectors at order G n+1 [51].Nevertheless, the present sector is still considerably more challenging than the corresponding non-spinning sector.The evaluation of the remaining contributions up to order G 3 that are required to complete the N 3 LO quadratic-in-spin sector should be facilitated with our extended upgrade of the EFTofPNG code [23,25], and this completion of the sector will be reported in forthcoming publications.
. Feynman graphs below three-loop order dependent on the spin-induced quadrupole, which contribute to the N 3 LO quadratic-in-spin static interaction at order G 4 .This is the only contribution to the sector with the spin-induced quadrupole.

Figure 4 .
Figure 4. Feynman graphs below three-loop order in the worldline picture, which contribute to the N 3 LO spin 1 -spin 1 static interaction at order G 4 .

(
2 LO N 3 LO N 4 LO N 5 LO Figure 2. Feynman graphs below three-loop order in the worldline picture, which contribute to the N 3 LO spin 1 -spin 2 static interaction at order G 4 .All of the graphs in this figure and the following ones should be accompanied by their 'mirror' graphs, in which worldline labels are exchanged, namely 1 ↔ 2.Figure 3. Feynman graphs at three-loop order in the worldline picture, which contribute to the N 3 LO spin 1 -spin 2 static interaction at order G 4 .
Figure 5. Feynman graphs at three-loop order in the worldline picture, which contribute to the N 3 LO spin 1 -spin 1 static interaction at order G 4 .