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Supersymmetric R4 Actions and Quantum Corrections to Superspace Torsion Constraints

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Supersymmetric R4 Actions and Quantum Corrections to Superspace Torsion Constraints DAMTP-2000-91, NORDITA-2000/87 HE, SPHT-T00/117, hep-th/0010182 SUPERSYMMETRIC R4 ACTIONS AND QUANTUM CORRECTIONS TO SUPERSPACE TORSION CONSTRAINTS K. Peetersa, P. Vanhoveb and A. Westerbergc a CERN, TH-division 1211 Geneva 23, Switzerland b SPHT, Orme des Merisiers, CEA / Saclay, 91191 Gif-sur-Yvette, France c NORDITA, Blegdamsvej 17, DK-2100 Copenhagen Ø, Denmark k.peeters, [email protected], [email protected] We present the supersymmetrisation of the anomaly-related R4 term in eleven dimensions and show that it induces no non-trivial modifications to the on-shell supertranslation algebra and the superspace torsion constraints before inclusion of gauge-field terms.1 1 Higher-derivative corrections and supersymmetry The low-energy supergravity limits of superstring theory as well as D-brane effective actions receive infinite sets of correction terms, proportional to in- 2 creasing powers of α0 = ls and induced by superstring theory massless and massive modes. At present, eleven-dimensional supergravity lacks a corre- sponding microscopic underpinning that could similarly justify the presence of higher-derivative corrections to the classical Cremmer-Julia-Scherk action [1]. Nevertheless, some corrections of this kind are calculable from unitarity argu- ments and super-Ward identities in the massless sector of the theory [2] or by anomaly cancellation arguments [3, 4]. Supersymmetry puts severe constraints on higher-derivative corrections. For example, it forbids the appearance of certain corrections (like, e.g, R3 corrections to supergravity effective actions [5]), and groups terms into var- ious invariants [6–9]. The structure of the invariants that contain anomaly- cancelling terms is of great importance due to the quantum nature of the 1Based on talks given by K.P. at the SPG meeting in Cambridge (February 2000) and in Groningen (September 2000), by A.W. at the Nordic Network Meeting in Copenhagen (May 2000), and by P.V. at the Fradkin Memorial Conference in Moscow (June 2000) and at the ARW Conference in Kiev (September 2000). 1 anomaly-cancellation mechanism and is the main concern of this note. Higher-derivative additions to the supergravity actions are in general com- patible with supersymmetry only if the transformation rules for the fields also receive higher-derivative corrections: n n δ + (α0) δ S + (α0) S =0: (1) 0 n 0 n Xn Xn As a consequence, the field-dependent structure coefficients on the right-hand side of the supersymmetry algebra, susy susy translation susy gauge Lorentz [δ1 ,δ2 ]=δ + δ + δ + δ ; (2) will be modified as well. When the theory is formulated in superspace the structure of the algebra is related to the structure of the tangent bundle, the link being provided by the constraints on the superspace torsion. In particular, corrections to the parameters modify the superspace constraints. However, since some corrections are reabsorbable by suitable rotations of the tangent bundle basis, not all corrections are physical. We report here on the supersymmetrisation of the anomaly-related terms 2 4 (α0) B F for super-Maxwell theory coupled to N=1 supergravity in ten ∧ 3 4 3 6 dimensions and (αM0 ) C t8R (where (αM0 ) =4π (lP ) ) in eleven dimensions performed in [10]. While∧ the former does not require any corrections to the superspace constraints, there are strong indications based on a previous super- space analysis [20] that the latter does induce such modifications. However, we show that there are no such corrections which are proportional to (powers of) the Weyl tensor only. We present here only the more salients aspect of the analysis and refer to the article [10] for computational and bibliographical details. Our main motivation to look for non-trivial corrections to superspace con- straints comes from the link between these constraints and the kappa symmetry of M-branes [11–13] and D-branes [14–16]. Classical kappa invariance of the M- and D-brane world-volume actions — a key requirement for these objects to be supersymmetric — imposes the on-shell constraints on the background superspace supergravity fields, among them the superspace torsion. For this reason, any non-trivial modification to the constraints is expected to require new terms in the world-volume actions for the branes in order for kappa sym- metry to be preserved. 2 2 Construction of an abelian F 4 superinvariant in D=10 As a first step in our analysis of the implications of higher-derivative correc- tions to the supersymmetry algebra, we discuss the construction of the abelian 2 4 4 (α0) (t8F B F ) for N=1 super-Maxwell theory coupled to gravity in ten dimensions.− ∧ The field content of the on-shell super-Maxwell theory comprises an abelian vector Aµ and a negative-chirality Majorana-Weyl spinor χ.Sinceweare interested in local supersymmetry invariance we have to take into account r also the interactions with the zehnbein eµ , the negative-chirality Majorana- Weyl gravitino µ and the two-form Bµν from the supergravity multiplet. The classical action (leaving out the gravitational sector) 10 1 µν µ νρ S 2 = d xe Fµν F 8¯χ D(!)χ +2¯χΓ Γ µ Fνρ (3) F Z − 4 − 6 is invariant under the local supersymmetry transformations δA = 4¯Γ χ, δχ= 1 Γµν F : (4) µ − µ 8 µν For local supersymmetry we have to consider the transformations of the super- gravity multiplet fields as well (neglecting terms proportional to the two-form Bµν and the corresponding field strength, Hµνρ): r r δe =2¯Γ ,δ = D (!) + ,δB=2¯Γ[ ] : (5) µ µ µ µ ··· µν µ ν The F 4 action invariant under the local supersymmetry transformations listed above has been determined previously [7, 8] and extends the globally super- symmetric action of [17, 18]. Using additional string input, we have managed to group all terms (including the fermionic bilinears) in a very compact way using the well-known t8-tensor [10]. The result is 2 (α0) 10 1 (r) 1 (r) 4 SF = d x 6 et8 Fr1r2 Fr7r8 + 12 "10 Br1r2 Fr3r4 Fr9r10 32 Z h ··· ··· 32 (r) 12 32 r1m r2 et η (¯χΓ D (!)χ)F F + · e (¯χΓ D (!)χ)F F − 5 8 r2r3 r1 r4 r5r6 r7r8 5 r1 r2 m 16 (r) 16 (r) ¯ "10 (¯χΓr1 r5 Dr6 (!)χ)Fr7r8 Fr9r10 + et8 ( r1 Γr2 χ)Fr3r4 Fr5r6 Fr7r8 − 5! ··· 3 8 ¯ mr1 r6 + 3 e ( mΓ ··· χ)Fr1r2 Fr5r6 : ··· i (6) 3 The local supersymmetry invariance of the combined action SF 2 +SF 4 requires that the supersymmetry transformations be modified according to (F 2 := mn F Fnm) 2 1 2 m 2 1 r1 r4 δAµ = 4¯Γµχ (α0) 4 (¯Γµχ)F (¯Γ χ)Fmµ 8 (¯Γ ··· µχ)Fr1r2 Fr3r4 ; − − h − − i 1 µν 1 2 (r) r1 r6 δχ = 8 Γ Fµν + 768 (α0) t8 Γr7r8 Γ ··· Fr1r2 Fr3r4 Fr5r6 : h − i (7) It can be verified that the structure of the supersymmetry algebra is not mod- 2 ified by the order-(α0) corrections [17,18,10]: (α )0 (α )2 (α )0 (α )2 (α )0 (α )0 4 δ 0 + δ 0 ,δ 0 + δ 0 A = δ 0 ,δ 0 A + (α0) : (8) 1 1 2 2 µ 1 2 µ O Consequently, the structure of the superspace torsion constraints will be the same as for the classical theory to this order. This observation is related to the fact that it is possible to supersymmetrise the Dirac-Born-Infeld actions while imposing only the classical constraints [19]. 3 Construction of the C R4 superinvariant in D=11 ∧ Noticing the close parallel between the classical supersymmetry transforma- tions for the super-Maxwell and the supergravity fields δχ = 1 Γµν F ,δ = 1 Γµν R + ; 8 µν rs 8 µνrs ··· δF = 8D (¯Γ χ) ,δRrs = 8D (¯Γ rs) (9) µν − [µ ν] µν − [µ ν] +4D (¯Γ rs +2¯Γ[r s] )+ ; [µ ν] ν] ··· it is tempting to make the following substitution in the super-Maxwell action: F R ,χ ;Dχ D ; (10) r1r2 → r1r2s1s2 → s1s2 r → r s1s2 Unfortunately, the difference in structure between the equations of motion for the gauge potential and the spin connection implies that the previous mapping does not commute with supersymmetry, as can be seen by the presence of the second line in the supersymmetry transformation of the Riemann tensor above. Another crucial difference between the super-Maxwell and supergravity cases is that, when subtracting all the lowest-order equations of motions, it is necessary to make the following substitution for the Riemann tensor: pq pq 16 [p ¯ r q] ¯ r q] Rmn Wmn δ[m ( r Γ| | n] | |Γ n]r) : (11) → − d 2 | | − − 4 Taking all these facts into account, as well as the information from string- amplitude analysis that the extra s-type indices in (10) should be contracted (s) 4 with an additional t8 tensor, we arrive at the following M-theory C R invariant after lifting to eleven dimensions [10]: ∧ 3 1 (r) (s) (α0 )− [0] =+ et t W W M LΓ 192 8 8 r1r2s1s2 ··· r7r8s7s8 1 t1t2t3r1 r8 (s) + " ··· t C W W ; (48)2 8 t1t2t3 r1r2s1s2 ··· r7r8s7s8 3 (s) ¯ (α0 )− [1] = 4 et ( Γ D )W W M LΓ − 8 s1s2 r1 r2 s3s4 r1r3s5s6 r3r2s7s8 1 et(s)( ¯ Γ )W W W − 4 8 r1 r2 s7s8 r1r2s1s2 mns3s4 nms5s6 et(s)( ¯ Γ )W W W − 8 r1 r2 s7s8 r1ms1s2 mns3s4 nr2s5s6 (s) ¯ + et8 ( r1 Γs7 r2s8 )Wr1r2s1s2 Wmns3s4 Wnms5s6 4 et(s)( ¯ Γ )W W W − 8 r1 s7 r2s8 r1ms1s2 mns3s4 nr2s5s6 2 (s) ¯ (12) + 9 et8 ( mΓn ms8 )Wpqs1s2 Wqps3s4 Wns7s5s6 8 et(s)( ¯ Γ )W W W ; − 9 8 m n ms8 nps1s2 pqs3s4 qs7s5s6 3 (s) ¯ (α0 )− [3] =+ 2et ( Γ D )W W M LΓ 8 s5s6 r1r2r3 r4 s7s8 r1r2s1s2 r3r4s3s4 ( ) 1 et s ( ¯ Γmr1r2 )W W W − 8 8 m s7s8 r1r2s1s2 pns3s4 nps5s6 1 (s) ¯ mr1r2 + 2 et8 ( mΓ s7s8 )Wr1ps1s2 Wpns3s4 Wnr2s5s6 (s) ¯ r1r2r3 + et8 ( mΓ s7s8 )Wr1r2s1s2 Wmns3s4 Wnr3s5s6 ; 3 1 (s) ¯r6 r1 r5 (α0 )− [5] =+ et ( Γ ··· )W W W ; M LΓ 8 8 s7s8 r1r2s1s2 r3r4s3s4 r5r6s5s6 3 1 (s) ¯ (αM0 )− Γ[7] =+ et8 ( mΓmr1 r6 s7s8 )Wr1r2s1s2 Wr3r4s3s4 Wr5r6s5s6 : L 48 ··· 3 Even though the elfbein supersymmetry transformation rule receives (αM0 ) modifications, by computing the closure of the supersymmetry algebra (2), we find [10] that the translation parameter does not receive corrections that cannot be absorbed by field redefinitions.
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