Superfield Approach to Nilpotency and Absolute Anticommutativity of Conserved Charges: 2D non-Abelian 1-Form Gauge Theory

We exploit the theoretical strength of augmented version of superfield approach (AVSA) to Becchi-Rouet-Stora-Tyutin (BRST) formalism to express the nilpotency and absolute anticommutativity properties of the (anti-)BRST and (anti-)co-BRST conserved charges for the two $(1+1)$-dimensional (2D) non-Abelian 1-form gauge theory (without any interaction with matter fields) in the language of superspace variables, their derivatives and suitable superfields. In the proof of absolute anticommutativity property, we invoke the strength of Curci-Ferrari (CF) condition for the (anti-)BRST charges. No such outside condition/restriction is required in the proof of absolute anticommutativity of the (anti-)co-BRST conserved charges. The latter observation (as well as other observations) connected with (anti-)co-BRST symmetries and corresponding conserved charges are novel results of our present investigation. We also discuss the (anti-)BRST and (anti-)co-BRST symmetry invariance of the appropriate Lagrangian densities within the framework of AVSA. In addition, we dwell a bit on the derivation of the above fermionic (nilpotent) symmetries by applying the AVSA to BRST formaism where only the (anti-)chiral superfields are used.


Introduction
The principle of local gauge invariance is at the heart of standard model of particle physics where there is a stunning degree of agreement between theory and experiment. One of the most elegant approaches to covariantly quantize the above kinds of gauge theories (based on the principle of local gauge invariance) is Becchi-Rouet-Stora-Tyutin (BRST) formalism where each local gauge symmetry is traded with two nilpotent symmetries which are christened as the BRST and anti-BRST symmetries. The latter symmetries are the quantum version of the gauge symmetries and their very existence ensures the covariant canonical quantization of a given gauge theory. The decisive features of the above quantum (anti-)BRST symmetries are the observations that (i) they are nilpotent of order two, and (ii) they are absolutely anticommuting in nature. In the language of theoretical physics, the nilpotency property ensures the fermionic (supersymmetic-type) nature of the (anti-)BRST symmetries and the linear independence of BRST and anti-BRST symmetries is encoded in the property of absolute anticommutativity of the above (anti-)BRST symmetries.
The superfield approach to BRST formalism [1][2][3][4][5][6][7][8] provides the geometrical basis for the properties of nilpotency and absolute anticommutativity that are associated with the (anti-)BRST symmetries. In the above usual superfield approach [1][2][3][4][5][6][7][8], the celebrated horizontality condition (HC) plays a key and decisive role. The HC leads, however, to the derivation (as well as geometrical interpretation) of the (anti-)BRST symmetries that are associated with the gauge and corresponding (anti-)ghost fields only . It does not shed any light on the (anti-)BRST symmetries that are associated with the matter fields in a given interacting gauge theory. In a set of papers [9][10][11][12], the above usual superfield formalism has been systematically generalized so as to derive the (anti-)BRST symmetries for the gauge, matter and (anti-)ghost fields together. The latter superfield approach [9][10][11][12] has been christened as the augmented version of superfield approach to BRST formalism where, consistent with the HC, additional restrictions (i.e. gauge invariant conditions) are also invoked. We shall exploit the latter superfield approach [9][10][11][12] to discuss a few key features of the 2D non-Abelian 1-form gauge theory (without any interaction with matter fields) that have already been discussed within the framework of BRST formalism [13][14][15][16].
To be more specific, in the above works [13][14][15][16], we have shown the existence of the nilpotent (anti-)BRST as well as (anti-)co-BRST symmetry transformations for the 2D non-Abelian 1-form gauge theory. The central theme of our present investigation is to capture the nilpotency and absolute anticommutativity of the (anti-)BRST and (anti-)co-BRST conserved charges [13][14][15][16] within the framework of augmented version of superfield approach (AVSA) to BRST formalism. In the proof of the absolute anticommutativity of the (anti-)BRST charges (within the framework of AVSA), we invoke the CF-condition to recast the expressions for these charges in an appropriate form and, then only, the superfield formalism is applied. However, in the case of the above proof of the (anti-)co-BRST charges, we do not invoke any CF-type restrictions. In our present investigation, we have proven the nilpotency and absolute anticommutativity of the conserved (anti-)BRST and (anti-) co-BRST charges that have been derived from two sets of coupled Lagrangian densities (cf. Eqs. (1), (39) below) for our 2D non-Abelian 1-form theory.
In the BRST approach to a given gauge theory, the existence of the (anti-)BRST symmetries and their conserved charges is well-known. However, we have been able to establish the existence of (anti-)co-BRST symmetry transformations (in addition to the nilpotent (anti-)BRST symmetry transformations) in the case of a toy model of a rigid rotor in one (0 + 1)-dimension of spacetime [17]. Furthermore, we have demonstrated the existence of such (i.e. (anti-)co-BRST) symmetries in the cases of Abelian p-form (p = 1, 2, 3) gauge theories in the two (1+1)-dimensions, four (3+1)-dimensions and six (5+1)-dimensions of spacetime (see, e.g., [18] and reference therein). In other words, we have established that the nilpotent (anti-)co-BRST symmetries exist for any arbitrary Abelian p-form (p = 1, 2, 3,...) gauge theory in D = 2p dimensions of spacetime [18]. One of the decisive features of the (anti-)co-BRST symmetries is the observation that it is the gauge-fixing term that remains invariant under these transformations (unlike the kinetic term that remains invariant under the (anti-)BRST transformations). The geometrical origin for these observations has been provided in our review article (see, e.g. [18] and reference therein).
We concentrate on the 2D non-Abelian theory (without any interaction with matter fields) because this theory has been shown [13] to be a perfect model of Hodge theory as well as a new model of topological field theory (TFT) which captures a few aspects of Wittentype TFTs [19] and some salient features of Schwarz-type TFTs [20]. The equivalence of the coupled Lagrangian densities of this 2D theory with respect to the (anti-)co-BRST symmetries has been established in our recent publication [14]. We have also discussed the CF-type restrictions for this theory within the framework of superfield approach [15] where we have demonstrated the existence of a tower of CF-type restrictions. This happens for this theory because it is a TFT where there are no physical propagating degrees of freedom for the 2D gauge field. In an another work [16], we have derived all the conserved currents and charges for this 2D theory and shown their algebraic structure that is found to be reminiscent of the Hodge algebra [21][22][23][24]. In other words, we have provided the physical realizations of the de Rham cohomological operators of differential geometry (and their algebra) in the language of the continuous (as well as discrete) symmetries, corresponding conserved charges and their algebra in operator form.
We have exploited the key ideas of AVSA to BRST formalism to derive the (anti-) BRST and (anti-)co-BRST symmetry transformations by using HC and dual-HC (DHC) as well as the (anti-)chiral superfield approach to BRST formalism (see, Appendices A and B below) in the context of our present 2D non-Abelian 1-form gauge theory. In our earlier works [9][10][11][12], we have never been able to capture the nilpotency as well as absolute anticommutativity properties of the (anti-)BRST and (anti-)co-BRST charges. The central objective of our present paper is to achieve this goal in the case of 2D non-Abelian 1-form gauge theory. To the best of our knowledge, this issue is being pursued for the first time in our present endeavor. Thus, the novelty in our present investigation is the observation that the nilpotency of the fermionic symmetry transformations and CF-type restrictions play a decisive role in capturing the nilpotency and absolute anticommutativity properties of the conserved (anti-)BRST and (anti-)co-BRST charges in the ordinary 2D spacetime (see, Sec. 5 below). However, it is the nilpotency of the translational generators (along the Grassmannian directions) that plays a crucial role for the same purpose within the framework of AVSA to BRST formalism on the supermanifold (see, Sec. 6 below).
The following key factors have spurred our curiosity to pursue our present investigation. First, to add some new ideas to the existing technique(s) of the superfield formalism is a challenging problem. In this context, we have expressed the fermionic charges (i.e. nilpotent (anti-)BRST and (anti-)co-BRST) charges in the language of the superfields and derivatives defined on the (2, 2)-dimensional supermanifold. Second, in our earlier works [14,15], we have derived the expressions for the conserved fermionic charges in the ordinary 2D space. It is a challenging problem to express their nilpotency and absolute anticommutativity properties in terms of the quantities that are defined on the (2, 2)-dimensional supermanifold. Third, it is also an interesting as well as novel idea to discuss various aspects of the (anti-)co-BRST charges within the framework of AVSA to BRST formalism. Finally, the insights and understandings, gained in our present investigation, would turn out to be useful when we shall discuss the 4D Abelian 2-form and 6D Abelian 3-form gauge theories within the framework of AVSA to BRST formalism. In fact, we have already shown, in our earlier works [25,26], that the above 4D and 6D Abelian 2-form and 3-form gauge theories are the models for the Hodge theory and they do support the existence of the (anti-)BRST and (anti-)co-BRST symmetries (as well as their corresponding conserved charges) in addition to the other continuous symmetries (and corresponding charges). There exist discrete symmetries, too, in these theories [25,26]. All these symmetries (and corresponding conserved charges) are required for the proof that the above models are the tractable field theoretic examples of Hodge theory.
Our present paper is organized as follows. In Sec. 2, we discuss the nilpotent (fermionic) (anti-)BRST and (anti-)co-BRST symmetries in the Lagrangian formulation. Our Sec. 3 is devoted to the discussion of horizontality condition (HC) that leads to the derivation of (anti-)BRST symmetries for the gauge field and corresponding fermionic (anti-)ghost fields along with the CF-condition. Sec. 4 of our paper deals with the dual-HC (DHC) which enables us to derive the (anti-)co-BRST symmetries that exist for the 2D non-Abelian 1-form gauge theory. The subject matter of Sec. 5 concerns itself with the discussion of nilpotency and absolute anticommutativity properties of the fermionic charges within the framework of BRST formalism in 2D ordinary spacetime. In Sec. 6, we discuss the nilpotency and absolute anticommutativity of the fermionic charges within the framework of AVSA to BRST formalism on a (2, 2)-dimensional supermanifold where the CF-condition plays an important role for (anti-)BRST charges. Finally, we discuss the key results of our present investigation in Sec. 7 where we point out a few possible theoretical directions which might be pursued for future investigations.
In our Appendices A and B, we derive the (anti-)BRST and (anti-)co-BRST symmetry transformations by exploiting the ideas of (anti-)chiral superfield approach to BRST formalism which match with the ones derived in the main body of the text. We express the (anti-)BRST and (anti-)co-BRST invariance of the Lagrangian densities in the language of the AVSA to BRST formalism in our Appendix C.
We note that the theoretical materials, contained in Secs. 5 and 6, are deeply interrelated. In fact, sometimes, it is due to our observations in Sec. 5 that we have been able to express the nilpotency and anticommutativity properties of the charges in Sec. 6 within the framework of AVSA to BRST formalism. On the other hand, at times, it is our knowledge of the AVSA to BRST formalism (cf. Sec. 6) that has turned out to be handy for our derivations of the above properties in 2D ordinary space (cf. Sec. 5).

Convention and Notations:
We take the 2D ordinary Minkowskian background spacetime to be flat with a metric tensor η µν = diag (+1, −1) where the Greek indices µ , ν , λ , ... = 0 , 1 correspond to the time and space directions, respectively. We choose 2D Levi-Civita tensor ε µν to obey the properties: ε µν ε µν = − 2!, ε µν ε νλ = δ λ µ , ε 01 = +1 = ε 10 , etc. In 2D, the curvature tensor (i.e. field strength tensor) F µν has only one existing component Here, in the SU(N) Lie algebraic space, we have adopted the notations A · B = A a B a and (A × B) a = f abc A b B c for the non-null vectors A a and B a where a, b, c = 1, 2, ....., N 2 − 1 and f abc are the structure constants in the SU(N) Lie algebra [T a , T b ] = f abc T c for the generators T a which are present in the definition of 1-form potential A µ = A µ · T = A a µ T a and curvature 2-form field strength tensor F µν = F µν · T = F a µν T a , etc. Through out the whole body of our text, we denote the (anti-)BRST and (anti-)co-BRST fermionic (s 2 (a)b = s 2 (a)d = 0) symmetry transformations by s (a)b and s (a)d , respectively.

Preliminaries: Nilpotent (Fermionic) Symmetries
We discuss here the (anti-)BRST and (anti-)co-BRST symmetries (and derive their corresponding conserved charges) in the Lagrangian formulation of the 2D non-Abelian 1-form gauge theory within the framework of BRST formalism. The starting coupled Lagrangian densities, in the Curci-Ferrari gauge [27,28], are: where B, B andB are the Nakanishi-Lautrup type auxiliary fields that have been invoked for various purposes. For instance, B is introduced in the theory to linearize the kinetic term (− 1 4 F µν · F µν = 1 2 E · E ≡ B · E -1 2 B · B) and auxiliary fields B andB satisfy the Curci-Ferrari restriction: B +B + (C ×C) = 0 where the (anti-)ghost fieldsC and C are fermionic (i.e. (C a ) 2 = (C a ) 2 = 0, C aC b +C b C a = 0, C a C b + C b C a = 0,C aC b +C bC a = 0,C a C b + C bC a = 0, etc.) in nature and they are required in the theory for the validity of unitarity. In the above, we have the covariant derivatives [D µ C = ∂ µ C + i (A µ × C) and D µC = ∂ µC + i (A µ ×C)] on the (anti-)ghost fields in the adjoint representation.
The Lagrangian densities in (1) respect the following off-shell nilpotent (s 2 (a)b = 0) (anti-)BRST symmetries transformations (s (a)b ) because the Lagrangian densities L B and LB transform under s (a)b as: It should be noted that both the Lagrangian densities in Eq. (1) respect both (i.e. BRST and anti-BRST) symmetries on the constrained hypersurface where the CF-condition (B +B + (C ×C) = 0) is satisfied. In other words, we note that because of the validity of CF-condition. As a consequence, the action integrals S = d 2 x L B and S = d 2 x LB remain invariant under the (anti-)BRST symmetries on the above hypersurface located in the 2D Minkowskian spacetime manifold. It is interesting to point out that the absolute anticommutativity {s b , s ab } = 0 is also satisfied on the above hypersurface which is defined by the field equation: B +B + (C ×C) = 0. According to the celebrated Noether's theorem, the above continuous symmetries lead to the derivations of conserved currents and charges. These (anti-)BRST charges, corresponding to the above continuous symmetries s (a)b , are (see, e.g. [14] for details) where a single dot on a field denotes the ordinary time derivative (e.g.Ċ = ∂ C/∂ t).
The above conserved charges Q (a)b are nilpotent (Q 2 b = Q 2 ab = 0) of order two and they obey absolute anticommutativity property (i.e. Q b Q ab + Q ab Q b = 0). These properties can be mathematically expressed as follows: The preciseness of the above expressions can be verified by taking into account the nilpotent (anti-)BRST symmetry transformation s (a)b (cf. Eq. (2)) and expressions for the nilpotent (anti-)BRST charges from Eq. (4). It should be noted that the property of absolute anticommutativity of the (anti-)BRST charges (i.e. {Q b , Q ab } = 0) is true only when we use the CF-condition (i.e. B +B + (C ×C) = 0).
The Lagrangian densities (1) also respect the following off-shell nilpotent ( s 2 (a)d = 0) and absolutely anticommuting (s d s ad + s ad s d = 0) (anti-)co-BRST [i.e. (anti-)dual BRST] symmetry transformations (s (a)d ) (see, e.g. [13], [14]) because the above Lagrangian densities transform, under s (a)d , as follows: It is clear that both the Lagrangian densities respect both (i.e. co-BRST and anti-co-BRST) fermionic symmetry transformations on a hypersurface where the CF-type restrictions B × C = 0, B ×C = 0 are satisfied. We lay emphasis on the observation that absolute anticommutativity {s d , s ad } = 0 is satisfied without any use of CF-type restrictions B ×C = 0, B ×C = 0. More elaborate discussions about these CF-type restrictions (and other related restrictions) can be found in our earlier works (see, e.g., [14,16] for details). The Noether conserved (Q (a)d = 0) charges Q (a)d , corresponding to the continuous and nilpotent symmetry transformations (6), are: The above charges are found to be nilpotent (Q 2 (a)d = 0) and absolutely anticommuting (Q d Q ad + Q ad Q d = 0) in nature. These claims can be verified in a straightforward fashion by taking the help of symmetries (6) and expressions of the charges (8) as follows: In fact, in this simple proof, one has to verify the l.h.s. of the above equations. In the forthcoming sections, we shall exploit the beauty and strength of the AVSA to BRST formalism to capture the above properties in a cogent and consistent manner.

Horizontality Condition: Off-Shell Nilpotent (Anti-)BRST Symmetry Transformations
We concisely mention here the key points associated with the geometrical origin of the nilpotent (anti-)BRST symmetries and existence of the CF-condition within the framework of Banora-Tonin (BT) superfield formalism [4,5]. In this connection, first of all, we generalize the 2D ordinary theory onto (2, 2)-dimensional supermanifold where the non-Abelian 1-form gauge field A µ (x) and (anti-)ghost fields (C)C are generalized onto their corresponding superfields with the following expansions (incorporating the secondary fields R µ ,R µ , S µ , B 1 , B 2 ,B 1 ,B 2 , s,s) on the (2, 2)-dimensional supermanifolds [4,5]: where the supermanifold is characterized by the superspace coordinates Z M = (x µ , θ,θ). The 2D ordinary bosonic coordinates x µ (µ = 0, 1) and the Grassmannian coordinates (θ,θ) (with θ 2 =θ 2 = θθ +θθ = 0) specify the superspace coordinate Z M and all the superfields, defined on the supermanifold, are function of them. The super curvature 2-form is where the super curvature tensorF M N = (F µν ,F µθ ,F µθ ,F θθ ,F θθ ,Fθθ). In the above equation, the ordinary exterior derivative d = dx µ ∂ µ and non-Abelian 1-form (A (1) = dx µ A µ ) gauge connection have been generalized onto the (2, 2)-dimensional supermanifold as where (∂ µ , ∂ θ , ∂θ) are the superspace derivatives (with ∂ µ = ∂ ∂x µ , ∂ θ = ∂ ∂θ and ∂θ = ∂ ∂θ ). We have observed earlier that the kinetic term (− 1 4 F µν · F µν = B · E − B·B 2 ) of the Lagrangian densities (1) remains invariant under the (anti-)BRST symmetries (2) and it has its origin in the exterior derivative d (i.e. F (2) (1) ). This gauge invariant quantity should remain independent of the Grassmannian variables (θ,θ) as the latter are only a mathematical artifacts and they cannot be physically realized. Thus, we have the following equality due to the gauge invariant restriction (GIR): The celebrated horizontality condition (HC) requires that the Grassmannian components of should be set equal to zero so that, ultimately, we should have the following equality, namely; The requirement of HC leads to the following [4,5,11,12] where the last entry is nothing but the celebrated CF-condition (B +B + (C ×C) = 0) if we identifyB 1 =B and B 2 = B. It is crystal clear that the HC leads to the derivation of the secondary fields in terms of the auxiliary and basic fields of the starting Lagrangian densities (1). The substitution of the above expressions for the secondary fields into the super expansion (10) leads to the following [4,5,11,12] where the superscript (h) on the superfields denotes the fact that these superfields have been obtained after the application of HC. A close look at the above expressions demonstrate that the coefficients of (θ,θ) are nothing but the anti-BRST and BRST transformations (2), respectively, that have been listed for the Lagrangian densities (1). Due to application of HC, ultimately, we obtain the following expression for the supercurvature tensor (as we have already setF µθ =F µθ =F θθ =F θθ =Fθθ = 0): Substitution of the expression for B which leads to the derivation of the (anti-)BRST symmetry transformations for the F µν (cf. (2)). It is now crystal clear that the requirements of gauge invariant restrictions in (14) and (13) are satisfied due to HC and, in this process, we have obtained the (anti-)BRST symmetry transformations for all the fields (as well as the CF-condition) for our theory.
We have derived these (anti-)BRST symmetry transformations by exploiting the potential of (anti-)chiral superfields approach to BRST formalism in our Appendix A.

Dual Horizontality Condition: Nilpotent (Anti-)co-BRST Symmetry Transformations
We exploit here the dual-HC (DHC) to derive the (anti-)co-BRST symmetry transformations for the (anti-)ghost fields and basic tenets of AVSA to obtain the precise form of the (anti-)co-BRST symmetry transformations associated with the gauge field (A µ = A µ · T ) of our 2D non-Abelian theory. In this context, first of all, we note that the gauge-fixing term (∂ µ A µ ) has its origin in the co-exterior derivative (δ = − * d * ) of the differential geometry in the following sense (see, e.g. [21][22][23][24] for details) where δ = − * d * is the co-exterior derivative and * is the Hodge duality operator on 2D Minkowskian flat spacetime manifold. It is clear that the Lorentz gauge-fixing term (∂ µ A µ ) is a 0-form which emerges out from the 1-form (A (1) = dx µ A µ ) due to application of the co-exterior derivative (δ = − * d * ) which reduces the degree of a form by one.
We have seen that the gauge-fixing term (∂ µ A µ ) remains invariant under the (anti-)co-BRST symmetry transformations (cf. Eq. (6)). We generalize this observation onto our chosen (2, 2)-dimensional supermanifold as follows whereδ is the super co-exterior derivative defined on the (2, 2)-dimensional supermanifold and ⋆ is the Hodge duality operator on the (2, 2)-dimensional supermanifold (see, e.g. [29] for details). The l.h.s. of (20) has already been computed in our previous work [29]. We quote here the result of operation ofδ onÃ (1) as 0-form, namely; where s θθ and sθθ appear in the following Hodge duality ⋆ operation: These factors (i.e. s θθ , sθθ) are essential to get back the 4-forms if we apply another ⋆ on (22). In other words, we have super Hodge duality ⋆ on the 0-form as follows: The equality in (21) ultimately, leads to because of the fact that there are no terms carrying the factors s θθ and sθθ on the r.h.s. At this stage, we substitute the expressions of B µ (x, θ,θ), F (x, θ,θ) andF (x, θ,θ) into Eq. (24) to derive the following important relationships: The last entry, in the above, is just like the CF-type restriction which is trivial. With the choices B 1 = −B andB 2 = B, we obtain the following expansions where the superscript (dh) denotes the expansions of the superfields after the application of DHC. It is self-evident that we have already obtained the (anti-)co-BRST symmetry transformation (4) for the (anti-)ghost fields (C)C of our theory as: Thus, the DHC leads to the derivation of (anti-)co-BRST symmetry transformations for the (anti-)ghost fields and very useful restrictions on the secondary fields in (25).
We are now in the position to derive the (anti-)co-BRST symmetry transformations s (a)d for the gauge field A µ . We exploit here the idea of AVSA to BRST formalism which states that the (anti-)co-BRST invariant quantities should be independent of the "soul" coordinates (θ,θ). During the early days of the developments of superspace technique, the bosonic coordinates x µ of the superspace coordinates Z M = (x µ , θ,θ) were called as the "body" coordinates and the Grassmannian variables (θ,θ) were christened as the "soul" coordinates. In this context, we observe that the following is true, namely; Thus, we have the following equality due to AVSA to BRST formalism: The substitution of the expansions from (26) yields the following: It is worthwhile to point out that we have not taken any super expansion of B(x) on the l.h.s. in (29) because of the fact that s (a)d B(x) = 0. In other words, we have taken . Ultimately, the relation in (30) produces the following: The substitution of these expressions into the super expansions of B µ (x, θ,θ) leads to the following (in terms of the (anti-)co-BRST symmetry transformations (6)): Here the superscript (dg) on B µ (x, θ,θ) denotes the expansion that has been obtained after the application of (anti-)co-BRST (i.e. dual gauge) invariant restriction (29). We end this section with the remark that we have obtained all the (anti-)co-BRST symmetry transformations for our 2D non-Abelian 1-form gauge theory by exploiting the theoretical strength of DHC and basic tenets of AVSA to BRST formalism.

Nilpotency and Absolute Anticommutativity of the Fermionic Charges: Ordinary 2D Spacetime
We, first of all, capture the nilpotency and absolute anticommutativity of the (anti-)BRST and (anti-)co-BRST charges in the ordinary space where the concepts/ideas behind the continuous symmetry and their generators (as well as the nilpotency of the (anti-)BRST and (anti-)co-BRST symmetry transformations) play very important roles. We would like to lay stress on the fact that some of the key results of our present section have been obtained due to our knowledge of the AVSA to BRST formalism that is contained in Sec. 6. Towards this goal in mind, we observe a few aspects of the conserved charges (listed in Eq. (4) and Eq. (8)) corresponding to the (anti-)BRST and (anti-)co-BRST symmetries of the Lagrangian densities (1). Using the (anti-)BRST and (anti-)co-BRST symmetry transformations of Eq. (2) and Eq. (6), we observe that the following are true, namely; It should be noted that we have expressed the conserved charges in (4) and (8) in terms of the transformations in Eqs. (2) and (6). It is elementary now to check that the nilpotency of the charges is satisfied due to the nilpotency properties of (anti-)BRST and (anti-)co-BRST symmetry transformations (i.e. s 2 (a)b = 0, s 2 (a)d = 0). In the above, we have used the basic principles behind the continuous symmetries and symmetry generators (as the conserved charges of the theory). We also point out that we have taken into account one of the expressions for Q (a)b and Q (a)d from Eq. (4) and Eq. (8) that have been explicitly derived in Sec. 2.
To prove the absolute anticommutativity properties of the (anti-)BRST and (anti-) co-BRST conserved charges, we note the following useful relationships which establish the absolute anticommutativity properties of the (anti-)co-BRST and nilpotent (anti-)BRST charges as follows due to, once again, the nilpotency (s 2 (a)b = 0, s 2 (a)d = 0) properties of the (anti-)BRST and (anti-)co-BRST symmetry transformations. It is interesting to point out that the expressions in the square brackets for the pair (Q b , Q ad ) and the pair (Q d , Q ab ) are exactly the same (as is evident from Eq. (35)). We would like to make a few remarks at this stage. A close look at equations (35) and (36) establishes one of the key observations that the nilpotency of symmetries and absolute anticommutativity properties of the conserved (anti-)BRST and (anti-)co-BRST charges are inter-related. Furthermore, we would like to mention that, in the expressions for Q (a)d in (35), we have dropped total space derivative terms in our computations. It is very important to emphasize here that in the expressions for Q (a)b (cf. Eq. (4)), we have utilized the strength of CF-condition (B +B + (C ×C) = 0) to recast these expressions in a suitable form before expressing them in the form (35). To elaborate on it, we take a simple example where the expression for the BRST charges Q b (cf. Eq. (4)), emerging from the Noether conserved current, is: Using the CF-condition B +B +(C ×C) = 0 (associated with the (anti-)BRST symmetries), we can recast the above expression in the following suitable form: The above form of the BRST charge has been expressed in the anti-BRST exact form as given in Eq. (35). A similar kind of argument has gone into the expression for the anti-BRST charge Q ab (cf. (35)) where we have been able to express it as the BRST exact form.
No such kinds of arguments have been invoked in the cases of the (anti-)co-BRST charges (cf. (35)) which have been expressed as the co-BRST exact and anti-co-BRST exact forms.
We have modified the Lagrangian densities (1) in our earlier works [14,16] by incorporating a couple of fermionic Lagrange multiplier fields (λ,λ with λ 2 =λ 2 = 0, λλ +λλ = 0) in such a manner that the following modified Lagrangian densities [14,16] respect the following perfect (anti-)co-BRST symmetries transformations: It can be checked that the above (anti-)co-BRST symmetry transformations are off-shell nilpotent and absolutely anticommuting in nature (where we do not invoke any kinds of CF-type restrictions for its validity). We also note that the superscripts (λ) and (λ) on the Lagrangian densities are logically correct because the Lagrange multipliers λ andλ characterize these Lagrangian densities. Furthermore, we observe that these Lagrange multiplier fields carry the ghost numbers equal to (+1) and (-1), respectively. Finally, it can be explicitly checked that the following are true, namely;  B ) would be different from (8). These conserved charges and their expressions have been derived in our earlier work (see, e.g. [16] for details). We quote here these expressions explicitly: In the above equivalent expressions, we have utilized the equations of motion (derived from the Lagrangian densities in Eq. (39)) and we have also dropped the total space derivative terms. To prove the nilpotency [(Q of the above charges, we note that they can be expressed in terms of the (anti-)co-BRST transformations as: The above expressions for the (anti-)co-BRST charges produce the last entry in the expres- Thus, we observe that the nilpotency of the charges Q ad = Q ad has already been proven in our present section itself. We note that the following are true: The above expressions demonstrate that the absolute anticommutativity property of the (anti-)co-BRST charges (i.e. {Q ad } = 0) is true and this property is primarily connected with the off-shell nilpotency (s 2 (a)d = 0) of the (anti-)co-BRST symmetry transformations (s (a)d ) that are present in our 2D non-Abelian theory (cf. Eq. (40)). To corroborate the above statements, it is straightforward to note that: From the above relationships, it is crystal clear that the absolute anticommutativity (i.e. {Q ad } = 0) for the (anti-)co-BRST charges is deeply connected with the nilpotency (s 2 (a)d = 0) property of the (anti-)co-BRST symmetry transformations (s (a)d ) for the Lagrangian densities (39). We wrap up this section with the remark that we have proven the nilpotency and absolute anticommutativity properties of the (anti-)co-BRST charges for the Lagrangian densities (1) as well as (39) where we do not invoke any kinds of CFtype restrictions. This observation is novel and drastically different from the proof of the absolute anticommutativity property of the conserved and nilpotent (anti-)BRST charges where it is mandatory for us to invoke the CF-condition. ,

Nilpotency and Absolute Anticommutativity of the Fermionic Charges: Superfield Approach
We express here the properties of nilpotency and absolute anticommutativity by exploiting the geometrical AVSA to BRST formalism. In this connection, first of all, we recall that the (anti-)BRST symmetry transformations s (a)b have been shown to be connected with the translational generators (∂ θ , ∂θ) along (θ,θ)-directions of the (2, 2)-dimensional supermanifold through the following mappings: We can very well choose the Grassmannian variables to be (θ 1 , θ 2 ) and identify the nilpotent symmetries: s b ↔ ∂ θ 1 | θ 2 =0 and s ab ↔ ∂ θ 2 | θ 1 =0 because there are other nilpotent (s 2 (a)d = 0) symmetries s (a)d in our theory, too. The latter nilpotent symmetries could be identified with translational generators as: s d ↔ ∂ θ 3 | θ 4 =0 and s ad ↔ ∂ θ 4 | θ 3 =0 where we shall have another set of a pair of Grassmannian variables (θ 3 , θ 4 ). However, for the sake of brevity, we have chosen only (θ,θ) as the Grassmannian variables so that we could discuss the (anti-)BRST and (anti-)co-BRST symmetries, separately and independently. The above mappings imply that the nilpotency of the (anti-)BRST symmetries (i.e. s 2 (a)b = 0) is intimately connected with the nilpotency (∂ 2 θ = ∂ 2 θ = 0) of the translational generators (∂ θ , ∂θ). This observation is utilized in expressing the expressions for the conserved and nilpotent (anti-)BRST charges in (33) as follows: The above expressions establish the nilpotency of the (anti-)BRST charges Q (a)b because: It should be noted that we do not invoke any kinds of CF-type restrictions for the proof of off-shell nilpotency of the above (anti-)BRST charges.
We capture now the absolute anticommutativity property of the (anti-)BRST symmetry generators Q (a)b in the language of the AVSA to BRST formalism. In this context, we concentrate on the expressions for (anti-)BRST charges that have been quoted in (35). It can be checked that we have the following expressions for these charges in the language of the AVSA to BRST formalism, namely; It is straightforward to note that the nilpotency properties of the translational generators (∂ θ , ∂θ) along the Grassmannian directions imply that: The above observations lead us to draw the conclusion that the absolute anticommutativity (Q b Q ab + Q ab Q b = 0) of the (anti-)BRST charges (cf. Eq. (36)) in the ordinary space can be captured in the language of the superfield approach to BRST formalism. We briefly comment here on the expressions for the (anti-)co-BRST charges Q (a)d that have been expressed in two different ways in Eq. (33) and Eq. (35). We have established earlier that the following mappings are true in the cases of s d and s ad : We can very well repeat here the previous footnote written in our manuscript. However, this would be only an academic exercise. The main issue is the fact that we discuss the (anti-)BRST and (anti-)co-BRST symmetries, within the framework of AVSA to BRST formalism, separately and independently. Thus, when we focus on (θ 1 , θ 2 ), we do not bother about (θ 3 , θ 4 ) and vice-versa. This is precisely the reason that we have taken, for the sake of brevity, only the (2, 2)-dimensional supermanifold for our discussion where, at a time, only a pair of Grassmannian variables are taken into account. Thus, the nilpotency of the (anti-)co-BRST charges can be expressed in terms of the quantities on the (2, 2)dimensional supermanifold as follows: where the superscript (dg) denotes the superfields (cf. Eq. (32)) that have been obtained after the application of (anti-)co-BRST invariant restriction in Eq. (29). Similarly, we note that the following is correct, namely; It is crystal clear, from Eqs. (53) and (54), that the following are true: The above relationships, in the ordinary 2D space, correspond to the following explicit expressions in the language of anticommutators: Thus, we have captured the nilpotency property of the (anti-)co-BRST charges in the language of the quantities that are defined on the (2, 2)-dimensional supermanifold. In fact, the nilpotency (Q 2 (a)d = 0) of the (anti-)co-BRST charges is deeply connected with the nilpotency (∂ 2 θ = 0, ∂ 2 θ = 0) of the translational generators (∂ θ , ∂θ) along the Grassmannian directions (θ,θ) of the (2, 2)-dimensional supermanifold.
Now we dwell a bit on the absolute anticommutativity property of the (anti-)co-BRST charges Q (a)d that have been expressed in Eq. (35). Taking the inputs from Eqs. (52), (32) and (26), we have the following Thus, the expressions for the (anti-)co-BRST charges (cf. Eq. (57)) imply The above expressions capture the absolute anticommutativity property of the (anti-)co-BRST charge (i.e. {Q d , Q ad } = 0) in the language of AVSA to BRST formalism. We observe, once again, it is the nilpotency (∂ 2 θ = ∂ 2 θ = 0) of the translational generators (∂ θ , ∂θ) that plays a decisive role in capturing the nilpotency as well as absolute anticommutativity properties of the (anti-)co-BRST charges in the terminology of AVSA to BRST formalism.
Finally, we would like to comment briefly on the nilpotency and absolute anticommutativity properties of the (anti-)co-BRST charges (Q ad ) that have been derived from the Lagrangian densities (39) and listed in (42) in different forms. We would like to lay emphasis on the fact that the Lagrangian densities (39) are very special in the sense that these Lagrangian densities respect proper (anti-)co-BRST symmetry transformations (listed in Eq. (40)) separately and independently (cf. Eq. (41)) where we do not invoke any kinds of CF-type restrictions from outside. Thus, as far as symmetry considerations are concerned, these Lagrangian densities are really beautiful from the point of view of the proper (anti-)co-BRST symmetry transformations (41). Within the framework of AVSA to BRST formalism, it can be checked that the expressions in (43) are: where the superfields with superscripts (dh) and (dg) have been explained in Sec. 4. It is clear, from the above expressions, that we have the following: The above relations prove the nilpotency of Q (λ) ad which is also connected with the nilpotency of the translational generators (∂ θ , ∂θ) along the Grassmannian directions (θ,θ) of the (2, 2)-dimensional supermanifold on which our 2D ordinary theory is considered.
To be more precise, the nilpotency of the above (anti-)co-BRST charges (which have been derived from the Lagrangian densities (39)) becomes very transparent when concentrating on the third and sixth lines in (60). In particular, the anticommutator of the conserved charges with themselves being zero immediately implies the nilpotency property (of these conserved charges). Let us now concentrate on the forms of the (anti-)co-BRST charges that have been written in Eq. (45). As is evident from Eq. (46), the absolute anticommutativity property of the (anti-)co-BRST charges is primarily hidden in Eq. (45) and is deeply connected with the nilpotency property of the (anti-)co-BRST symmetry transformations (s (a)d ). Thus, we express the forms of the (anti-)co-BRST charges (45) in the language of AVSA to BRST formalism as follows where the superfields with superscripts (dh) and (dg) have already been explained in Sec. 4. It is straightforward to note, from the above equation, that: We end this section with the remark that the absolute anticommutativity property of the (anti-)co-BRST charges is deeply connected with the nilpotency property (∂ 2 θ = ∂ 2 θ = 0) of the translational generators (∂ θ , ∂θ) along the Grassmannian directions (θ,θ) of the (2, 2)-dimensional supermanifold on which our 2D ordinary non-Abelian theory is generalized.

Conclusions
We have exploited the theoretical strength of the AVSA to BRST formalism to express the properties of the nilpotency and absolute anticommutativity of the fermionic conserved charges (i.e. (anti-)BRST and (anti-)co-BRST charges) of our self-interacting 2D non-Abelian theory (without any interaction with matter fields). We have not achieved this goal in our earlier works [9][10][11][12] on the AVSA to BRST formalism. Thus, the results in our present investigation are achieved for the first time. It is straightforward to express the nilpotency property of the fermionic (i.e. conserved (anti-)BRST and (anti-)co-BRST) charges in the language of the AVSA to BRST formalism. However, the property of absolute anticommutativity is captured, within the framework of AVSA to BRST formalism, by applying specific mathematical trick where the CF-condition plays a decisive role.
We would like to lay emphasis on the contents of Sec. 5 where we have been able to exploit the virtues of symmetry principles to express the (anti-)BRST and (anti-)co-BRST charges in various exact-forms. These theoretical expressions have been exploited, in turn, to capture the nilpotency and absolute anticommutativity properties in the language of AVSA to BRST formalism in Sec. 6. We observe that the CF-condition (B +B +(C ×C) = 0) enables us in expressing the BRST charge as an anti-BRST exact form and anti-BRST charge as a BRST exact form. We would like to lay emphasis on the fact that the contents of Secs. 5 and 6 are intertwined in an elegant manner. Though it appears, from our statements in this paragraph, that the contents of Sec. 5 have influenced our results in Sec. 6. However, we would like to stress that, many a times, our understandings of the contents of Sec. 6 have influenced our results in Sec. 5. Thus, to be precise, the key results of our present endeavor are influenced by our knowledge of both the above sections which are inter-related. These results play an important role in establishing the absolute anticommutativity properties of the above fermionic charges. Thus, first of all, we have proven the nilpotency and absolute anticommutativity of the (anti-)BRST and (anti-)co-BRST charges in the language of symmetry properties (cf. Sec. 5). In particular, we have shown that it is the nilpotency of the (anti-)BRST and (anti-)co-BRST symmetry transformations that has played a decisive role in the proof of the above properties in the ordinary 2D space of our non-Abelian 1-form gauge theory. In fact, the results of Sec. 5 have been translated into the language of AVSA to BRST formalism in Sec. 6.
The proof of the nilpotency and absolute anticommutativity properties in the language of AVSA to BRST formalism for the fermionic (anti-)BRST and (anti-)co-BRST charges is a novel result because, in our earlier works on AVSA to BRST formalism [9][10][11][12], we have not achieved this goal. In our very recent works [30][31][32], we have captured the property of the absolute anticommutativity of nilpotent charges within the framework of (anti-)chiral superfield approach to BRST formalism. However, we have not done so within the framework of AVSA to BRST formalism where the full expansions of the superfields are taken into account. We plan to exploit our present idea to consolidate it by applying it to the cases of 1D toy model of the rigid rotor, 2D self-dual bosonic theory, modified versions of 2D Proca and anomalous gauge theory, 4D Abelian 2-form and 6D Abelian 3-form gauge theories where we have demonstrated the existence of (anti-)BRST and (anti-)co-BRST charges as these theories are the models for the Hodge theory [18,[30][31][32].
Here we derive the (anti-)BRST symmetries (cf. Sec. 2) by exploiting the simple (but fruitful) augmented version of (anti-)chiral superfield approach (ACSA) to BRST formalism [30][31][32] where the (anti-)BRST invariant restrictions play very crucial roles. In this context, first of all, we generalize the basic 2D fields (e.g. A µ , C,C) onto (2, 1)-dimensional antichiral super-submanifold (of the general (2, 2)-dimensional supermanifold) as: which are nothing but the limiting cases of the super expansions in Eq. (10) (that are on the general (2, 2)-dimensional supermanifold). It is worthwhile to mention here that the Nakanishi-Lautrup auxiliary field B(x) has no anti-chiral expansion (i.e. B(x) →B(x,θ) = B(x)) because we note that s b B(x) = 0. We further point out that s b (C × B) = 0. This observation can be generalized onto the anti-chiral (2, 1)-dimensional super-submanifold with the following restriction on the superfields due to the ACSA to BRST formalism: which leads to B 2 × B = 0. One of the non-trivial solutions is B 2 is proportional to B. For the sake of brevity, however, we choose B 2 = B. The above restriction (A.2) is consistent with the basic tenets of AVSA/ACSA to BRST formalism where we demand that the BRST invariant quantity should be independent ofθ variable. Thus, we havē where the superscript (b) denotes that the superfieldF (b) (x,θ) has been obtained after the application of BRST invariant restriction (A.2). It goes without saying that (in the above process) we have derived the BRST transformation forC as: s bC = iB (cf. Sec. 2). We carry out the above kinds of exercises to obtain the other BRST symmetry transformations associated with the other fields of the theory. In this context, first of all, we observe that the following are the useful BRST-invariant quantities (in addition to the earlier BRST-invariant quantities: s b B = 0, s b (B ×C) = 0), namely; According to the AVSA/ACSA to BRST formalism, the above quantities can be generalized onto the (2, 1)-dimensional anti-chiral super-submanifold and the corresponding superfields can be restricted to obey the following conditions: In other words, we demand that the l.h.s. of the above equality should remain independent of "soul" coordinateθ. The above requirements lead to the following: We discuss here the solutions of the above conditions. It is clear that B 1 (x) is proportional to (C(x) × C(x)) because we have obtained the condition B 1 (x) × C(x) = 0 in (A.6). Thus, the non-trivial expression for B 1 (x) = κ (C(x) × C(x)) where κ is a numerical constant. From the relation D µ B 1 (x) + R µ (x) × C = 0, it is clear that the following choices satisfy the relation B 1 (x) × C(x) = 0 and D µ B 1 + (R µ × C) = 0 together. It is gratifying to note that these conditions also satisfy the last relationship that has been quoted in (A.6). Thus, ultimately, we have obtained the following expansions (with superscript (b)): In other words, we have already derived the BRST symmetry transformations s b for the basic fields (A µ , C,C) which are nothing but the coefficients ofθ in the superfields expansions (A.8). The sanctity of this statement can be checked from Eq. (2).
Finally, we comment on the derivation of the BRST symmetry transformations: s b B = i (B × C), s b E = i (E × C) and s bB = i (B × C). In this context, we have the following generalizations on the (2, 1)-dimensional anti-chiral super-submanifold: where (P (x), Q(x), S(x)) are the fermionic secondary fields which have to be determined in terms of the basic and auxiliary fields of the theory. We note the following: According to the basic tenets of AVSA/ACSA, we have the following equalities which show that the BRST invariant quantities of (A.10) should remain independent of the "soul" coordinateθ. This restriction yields the following: Thus, ultimately, we have derived the following: where superscript (b) denotes the fact that the above super expansions have been derived after the application of the BRST invariant restrictions (A.10) and (A.11). From Eq. (A.13), we note that coefficients ofθ are nothing but the BRST symmetry transformations for B, E andB fields as given in Eq. (2) (cf. Sec. 2 for details). We now focus on the derivation of the anti-BRST symmetry by chiral superfield approach to BRST formalism where we have the following generalizations: where (R µ ,B 1 ,B 2 ) are the secondary fields that have to be determined in terms of the basic and auxiliary fields of the theory by invoking the anti-BRST invariant restrictions. It goes without saying that the above expansions are the limiting cases of the super expansions in Eq. (10) whenθ = 0. It can be checked that we have the following useful and interesting anti-BRST invariant quantities (cf. Sec. 2): According to the basic tenets of AVSA/ACSA, we have to demand that the above quantities (when generalized onto (2, 1)-dimensional chiral supermanifold) should be independent of the Grassmannian variable θ. In other words, we have the following equalities: We note here that, because of s abB = 0, we have no chiral super expansion ofB(x) (i.e. B(x) −→B(x, θ) =B(x)). The above equalities lead to the following expressions for the secondary fields (R µ ,B 1 ,B 2 ) in terms of basic and auxiliary fields of our theory: Thus, we have obtained the following chiral super expansions According to the basic principles of AVSA/ACSA, the above quantities should be independent of the Grassmannian variable θ when they are generalized onto the (2, 1)-dimensional chiral super-submanifold. In other words, we have the following equalities where the expansion for the chiral superfieldF (ab) (x, θ) has been given in (A.18) and the chiral super expansions of the other superfields are as follows: Hence, the fields (P (x),Q(x),S(x)) are the fermionic secondary fields that are to be determined in terms of the basic and auxiliary fields of our 2D non-Abelian theory from the anti-BRST invariant restrictions (cf. (A.19), (A.20)). Explicit substitution of expansions from (A.18) and (A.21) lead to the following very useful and interesting relationships: These relationships prove the fermionic nature of the secondary fields (P (x),Q(x),S(x)) which is also evident from (A.21) due to the fermionic (θ 2 = 0) nature of θ. Thus, we have the following super expansions for the superfields in (A.21), namely; where the superscript (d) on the superfields denotes that the above superfields have been derived after the application of co-BRST invariant restrictions (B.1) which demonstrate that the co-BRST invariant quantities should be independent of the soul coordinateθ (due to the basic tenets of augmented version of (anti-)chiral superfield approach to BRST formalism). Further, the other co-BRST invariant quantities in (B.1) imply It is evident that the non-trivial co-BRST symmetry transformations are s d C = −iB and s d A µ = −ε µν ∂ νC . These can be derived from the co-BRST invariant restrictions: The substitution of the expansion of F (x,θ) from (A.1) into the top relationship, in the above, leads to the condition B 1 × B = 0. One of the non-trivial solution is B 1 = −B so that we obtain the following useful expansion: Finally, when we substitute the expansions for B µ (x,θ) from (A.1), B (d) (x,θ),F (d) (x,θ) from (B.2) and F (d) (x,θ) from (B.5), we obtain: R µ (x) = −ε µν ∂ νC which also satisfies both the additional conditions in (B.3) and leads to: The super expansions in (B.2), (B.5) and (B.6) demonstrate that we have derived: We mention, in passing, that s d B = 0 implies that we have no anti-chiral expansion for B(x) as it is a co-BRST invariant quantity.
To derive the anti-co-BRST symmetry transformations, we invoke the chiral expansions for the superfields as given in (A.14) and (A.20). In this context, first of all, we look for the useful anti-co-BRST invariant quantities and generalize them onto (2, 1)-dimensional chiral super submanifold (of the general (2, 2)-dimensional supermanifold on which our present theory is generalized). After this, we demand that such invariant quantities should be independent of the "soul" coordinate θ. In this context, we note the following: The trivial chiral expansions are: which imply s ad C = s ad B = s adB = s ad B = 0. The non-trivial conditions are: which imply that if we chooseB 2 = B, the conditionB 2 × B = 0 is satisfied and it leads tō where the superscript (ad) denotes that the above superfield has been obtained after the application of (B.7). Thus, we observe that we have already derived the non-trivial antico-BRST symmetry transformation: s adC = iB. We now focus on the latter conditions where we have to use F (ad) (x, θ) = C(x) and (B.9) to obtain the following conditions: Thus, ultimately, we obtain the chiral expansion: where the supersript (ad) denotes that the above superfield has been obtained after the application of (B.7). It is evident, by now, that we have obtained all the anti-co-BRST symmetry transformations s ad (cf. Sec. 2) of our theory by exploiting the symmetry invariant restrictions on the chiral superfields. We point out that the choice R µ = −ε µν ∂ ν C satisfies both the additional conditions ∂ µR µ = 0 andR µ × ∂ µ C = 0 which are present in (B.9) and (B.11). We comment that we have chosen B 1 = −B andB 2 = +B (which imply s d C = −iB and s adC = iB) because these choices satisfy the absolute anticommutativity property (s d s ad + s ad s d = 0) of the (anti-)co-BRST symmetry transformations.

Appendix C: On the Symmetry Invariance in the Theory
We have concentrated on the (anti-)BRST as well as (anti-)co-BRST invariance(s) of our present 2D non-Abelian theory within the framework of AVSA to BRST formalism. In this Appendix, we capture the (anti-)BRST and (anti-)co-BRST invariance of the Lagrangian densities (1) and (39) within the framework of AVSA to BRST formalism (which are explicitly quoted in Eqs. (3), (7) and (40)). Towards this goal in mind, first of all, we generalize the Lagrangian densities (1) onto (2, 2)-dimensional supermanifold as follows, where the superfields with superscript (h) are the ones that have been derived in the main body of the text. It is to be noted that we have defined the covariant derivatives as: x, θ,θ)). The superfields with superscript (g) denote the ones that have been obtained after GIR. We elaborate here a few of them. For instance, let us focus on the explicit expression of B (g) (x, θ,θ). In this context, we note that: At this stage, we exploit the basic tenets of AVSA to BRST formalism which state that any arbitrary (anti-)BRST invariant quantity must remain independent of the "soul" coordinates (θ,θ) when it is generalized onto an appropriately chosen supermanifold on which our basic gauge theory is generalized. Thus, we have the following equality: In the above, the full expansions for E (h) (x, θ,θ) and B(x, θ,θ) are where E (h) (x, θ,θ) has been derived from Eq. (18) and the general super expansion for the superfield B(x, θ,θ) has been quoted in (C.4) where the secondary fields (S(x),S(x)) are fermionic and P (x) is bosonic in nature. The substitution of (C.4) into (C.3) produces the following expressions for the secondary fields in terms of the basic and auxiliary fields: In other words, we have derived the (anti-)BRST symmetry transformations for the auxiliary field B(x) and, in the process, we have obtained the explicit form of B (g) (x, θ,θ) which has been used in the explicit expression for the super Lagrangian densities (C.1).
We are now in the position to express the (anti-)BRST invariance of the Lagrangian densities (1) which change to the total spacetime derivatives under the above symmetry transformations (cf. Eqs. (3), (4)). It is straightforward to check that which are nothing but our earlier results (cf. Eq. (3)) where we have shown that s ab LB = − (B · D µC ) and s b L B = ∂ µ (B · D µC ). Geometrically, the above observations show that super Lagrangian densities (C.1) are the sum of composite (super)fields, obtained after (anti-)BRST invariant restrictions and HC, such that their translation along the (θ,θ) directions of the (2, 2)-dimensional supermanifold produces the total spacetime derivatives.
(C. 16) We note that the substitution of the super expansions from Eqs. (26) and (32) into the super Lagrangian densities (C.14) would express them in terms of the coefficients of (1, θ,θ, θθ). It can be now checked that the following are true, namely; Hence, we have provided the equivalence of the (anti-)co-BRST invariance of the Lagrangian densities (1) in the language of AVSA to BRST formalism. Consequently, the (anti-)co-BRST invariance can be explained within the framework of AVSA to BRST formalism as follows. The translation of the super Lagrangian densities (C.14) along (θ,θ)-directions of the (2, 2)-dimensional supermanifold is such that it results in the total spacetime derivatives thereby rendering the action integrals (corresponding to the appropriate Lagrangian densities) invariant under the (anti-)co-BRST symmetry transformations. We end this Appendix with a concise remark that we can also capture the (anti-)co-BRST invariance of the coupled Lagrangian densities (39) exactly in the same manner as we have done for our starting Lagrangian densities (1) for the present 2D non-Abelian 1-form gauge theory.