ISSN: 2689-7636
##### Annals of Mathematics and Physics
Review Article       Open Access      Peer-Reviewed

# Poisson structures on (non)associative noncommutative algebras and integrable Kontsevich type Hamiltonian systems

### Oksana E Hentosh1, Alexander A Balinsky2 and Anatolij K Prykarpatski3*

1Institute for Applied Problems of Mechanics and Mathematics, NAS, Lviv, 79060 Ukraine
2Institute of Mathematics, Cardiff University, Cardiff CF24 4AG, Great Britain, UK
3Department of Physics, Mathematics and Computer Science, Cracov University of Technology, Krakow, Poland
*Corresponding author: Anatolij K Prykarpatski, Department of Physics, Mathematics and Computer Science, Cracov University of Technology, Krakow, Poland, E-mail: pryk.anat@cybergal.com
Received: 27 December, 2019 | Accepted: 29 January, 2020 | Published: 31 January, 2020
Keywords: Hamiltonian systems; Lie-Poisson structure; Group agebras; π-metrized Lie aleg-bras; Kontsevich type systems

Cite this as

Hentosh OE, Balinsky AA, Prykarpatski AK (2020) Poisson structures on (non)associative noncommutative algebras and integrable Kontsevich type Hamiltonian systems. Ann Math Phys 3(1): 001-006. DOI: 10.17352/amp.000010

We have revisited the classical Poisson manifold approach, closely related to construction of Hamiltonian operators, generated by nonassociative and noncommutative algebras. In particular, we presented its natural and simple generalization allowing effectively to describe a wide class of Lax type integrable nonlinear Kontsevich type Hamiltonian systems on associative noncommutative algebras.

### Introduction

We present a classical Poisson manifold approach, closely related to construction of integrable Hamiltonian systems, generated by nonassociative and noncommutative algebras. In particular, we devise its natural and simple generalization, useful for describing a wide class of Lax type integrable nonlinear Hamiltonian systems on associative noncommutative algebras, initiated first in [1-4], in case of the associative noncommutative operator algebras and continued later in [5-11], in case of general associative noncommutative algebras.

##### Poisson structures on non commutative functional manifolds

It is interesting to look at construction of the Hamiltonian operators and revisit it from the classical point of view, considering them as those defined on the naturally associated [4,12-17], cotangent space ${T}^{\ast }\left(M\right)$ to some linear functional noncommutative manifold M $\simeq {\stackrel{˜}{\mathbb{A}}}^{\ast }\simeq \stackrel{˜}{\mathbb{A}},$ where $\mathbb{A}$ is, in general, a (non)associative noncommutative algebra over a field $\mathbb{K}$ $\stackrel{˜}{\mathbb{A}}:={C}^{\infty }\left({\mathbb{S}}^{1};\mathbb{A}⋫$ , and $\stackrel{˜}{\mathbb{A}}$ is its naturally adjoint space. Then, a Hamiltonian operator on M is defined [12,15], as a smooth mapping $\vartheta :M\to Hom\left({T}^{\ast }\left(M\right);T\left(M\right)\right),$ such that for any fixed $u\in M$ the bracket

where $f,g:M\to \mathbb{K}$ are arbitrary smooth mappings from the functional space $\mathcal{D}\left(M\right)\simeq {ℱ}_{\stackrel{˜}{\mathbb{A}}}\left(u\right),$ satisfies the Jacobi identity. The bracket (2.1) is determined on M by means of the natural convolution $\left(\cdot ,\cdot \right)$ on the product ${T}^{\ast }\left(M\right)×T\left(M\right),$ and respectively, the gradient $\nabla f\left(u\right)\in {T}^{\ast }\left(M\right)$ of a function $f\in \mathcal{D}\left(M\right)$ is calculated as

for any $h\in T\left(M\right).$ It is well known [18,19], that a linear operator $\vartheta \left(u\right):{T}^{\ast }\left(M\right)\to T\left(M\right),$ determined at any point $u\in M,$ is Hamiltonian iff the suitably defined [18], Schouten–Nijenhuis bracket

identically on M Namely, this condition (2.3) was used in the investigations [18,20], to formulate criteria for the operator $\vartheta \left(u\right):{T}^{\ast }\left(M\right)\to T\left(M\right)$ to be Hamiltonian on the functional manifold M. Yet these criteria appear to be very complicated and involve a large amount of cumbersome calculations even in the case of fairly simple differential expressions. So, we have reanalyzed this problem from a slightly different point of view. First, recall that the Jacobi identity for the bracket (2.1) is completely equivalent to the fact that the bracket operator defined as ${D}_{f}\left(g\right):=\left\{f,g\right\}$ for a fixed $f\in \mathcal{D}\left(M\right)$ and arbitrary $g\text{\hspace{0.17em}}\in \mathcal{D}\left(M\right)$ acts as a derivation on the space $\left(\mathcal{D}\left(M\right);\left\{\cdot ,\cdot \right\}\right):$

where $g,h\in \mathcal{D}\left(M\right)$ are taken arbitrary. This can be easily reformulated as follows: take any element $\phi \in {T}^{\ast }\left(M\right),$ such that the Fréchet derivative ${\phi }^{\text{'}}\left(u\right)={\phi }^{\text{'},\ast }\left(u\right)$ at any $u\in M$ with respect to the convolution $\left(\cdot ,\cdot \right)$ on ${T}^{\ast }\left(M\right)×T\left(M\right),$ and construct a vector field $K:M\to T\left(M\right)$ as

Then the derivation condition (2.4) can be equivalently rewritten [4,12,15-17], as the strong Lie derivative

along the vector field $K\left(u\right)=\vartheta \left(u\right)\phi \left(u\right)\in T\left(M\right)$ at any $u\in M$ for all “self-adjoint” elements $\phi \in {T}^{\ast }\left(M\right).$ Equivalently, a given linear skew-symmetric operator $\vartheta \left(u\right):{T}^{\ast }\left(M\right)\to T\left(M\right),u\in M,$ is Hamiltonian iff the Lie derivative (2.6) vanishes for all “self-adjoint” elements $\phi \in {T}^{\ast }\left(M\right).$ Moreover, as was observed in [21], it suffices to check the condition (2.6) only on the subspace of elements $\phi \in {T}^{\ast }\left(M\right)$ satisfying the condition ${\phi }^{\text{'}}\left(u\right)=0$ for any $u\in M.$

As an example, one can check that a skew-symmetric matrix-differential operator on M of the form

where, an -dimensional square matrix $\sigma \left(u\right):=\left(\sum _{s=1}^{n}{u}_{s}{\sigma }_{ij}^{s}:i,j=\overline{1,n},n\in {ℤ}_{+}\right),\text{\hspace{0.17em}}u\in M,$ satisfies the condition (2.6) iff the linearly independent elements from $\underset{\mathbb{K}}{span}\left\{{e}_{j}\in \mathbb{A}:j=\overline{1,n}\right\}$ generate the finite dimensional nonassociative Balinsky-Novikov algebra [22] and satisfy the conditions ${e}_{i}\circ {e}_{j}=\sum _{s=1}^{n}{\sigma }_{ij}^{s}{e}_{s}$ for all $i,j=\overline{1,n}.$ Similarly, one can verify that the skew-symmetric inverse-differential operator

where, as above $\sigma \left(u\right):=\left(\sum _{s=1}^{n}{u}_{s}{\sigma }_{ij}^{s}:u\in M,i,j=\overline{1,n},n\in {ℤ}_{+}\right),$ the sign $"⊺"$ means the usual matrix transposition, is Hamiltonian iff the basic nonassociative algebra $\mathbb{A}:\underset{\mathbb{K}}{span}\left\{{e}_{j}:j=\overline{1,n}\right\}$ coincides with the right Leibniz algebra [23] and the condition ${e}_{i}\circ {e}_{j}=\sum _{s=1}^{n}{\sigma }_{ij}^{s}{e}_{s}$ holds for any $i,j=\overline{1,n}\text{\hspace{0.17em}}$ . The skew-symmetric inverse-differential operator (2.8) can be naturally generalized to the expression

which can be rewritten as

where, by definition, ${D}_{x}{D}_{x}^{-1}=I$ and ${D}_{x}^{-1}\left(...\right):=\frac{1}{2}\left[{\int }_{0}^{s}ds\left(...\right)-{\int }_{s}^{2\pi }ds\left(...\right)\right]$ for all $x\in 0,2\pi \right].$ The condition (2.6) for the operator (2.10) to be Hamiltonian reduces to the constraints on the related nonassociative algebra $\mathbb{A}:\underset{\mathbb{K}}{span}\left\{{e}_{j}:j=\overline{1,n}\right\}\text{\hspace{0.17em}}$ exactly coinciding with those, analyzed in some detail in [24] .

As it was already mentioned [18,24], based on the matrix representations of the right Leibniz algebra and the new nonassociative Riemann algebra, one can construct many nontrivial Hamiltonian operators $\vartheta \left(u\right):{ℒ}_{\stackrel{˜}{\mathbb{A}}}\to {ℒ}_{\stackrel{˜}{\mathbb{A}}}^{\ast }$ on the adjacent weak Lie algebra ${ℒ}_{\stackrel{˜}{\mathbb{A}}},$ related with diverse types of nonassociative noncommutative algebras $\mathbb{A}.$ These Hamiltonian operators prove to be very useful [25,26,27], for describing a wide class of multicomponent hierarchies of integrable Riemann type hydrodynamic systems and their various physically reasonable reductions.

##### Poisson structures on manifolds generated by associative non commutative algebras

Proceed now to a slightly generalized construction of Hamiltonian operators on a phase space, generated by associative noncommutative algebra A-valued matrices, which was first studied in [1-4], in case of the noncommutative operator algebras and continued later in [5-11], in case of general associative noncommutative algebras. This natural and simple generalization appeared to be very useful [28,29,30,31,8-10], for describing a wide class of new Lax type integrable nonlinear Hamiltonian systems on associative noncommutative algebras, interesting for diverse applications in modern quantum physics.

We start here with a free associative noncommutative algebra $A=\mathbb{K}{u}_{1},{u}_{2},...,{u}_{m}>,$ generated by a finite set of elements $\left\{{u}_{j}\in A:j=\overline{1,m}\right\},$ and define its “abelianization” ${A}_{♮}:=A/\left[A,A\right]$ and the projection $\pi :A\to {A}_{♮},\text{\hspace{0.17em}}$ where the space $\left[A,A\right]:=$ $\left\{uv-vu\in A$ $:u,v\in A\right\}.$ Consider now a naturally related with A n-dimensional matrix Lie algebra $\mathcal{G}:=gl\left(n;A\right)$ over the field $\mathbb{K}$ with entries in A subject to the usual matrix commutator $\left[\text{a,b}\right]:=\text{ab}-\text{ba}\text{\hspace{0.17em}}$ for all $\text{a,b}\in \mathcal{G}.$ Being first interested in the Lie-algebraic studying [14,15,32,33], of co-adjont orbits on the adjoint space ${\mathcal{G}}^{\ast },$ let us construct a bi-linear form $<\cdot |\cdot >:\mathcal{G}×\mathcal{G}\to {A}_{♮}$ on the Lie algebra $\mathcal{G}$ by means of the trace-type expression

for any $\text{a},\text{b}\in \mathcal{G}.$ The following important lemma holds.

Lemma 3.1 The bilinear form (3.1) on $\mathcal{G}$ is symmetric, nondegenerate and ad-invariant.

Proof. Symmetricity: We have:

for any $\text{a,b}\in \mathcal{G}.$

Nondegeneracy: Assume that $<\text{a|b}{>=0}_{♮}\in {A}_{♮}$ for a fixed $\text{a}\in \mathcal{G}$ and all $\text{b}\in \mathcal{G}.$ state that $\text{a=0,}$ let us put then $\text{b=a}\text{\hspace{0.17em}}\text{\hspace{0.17em}}$ and obtain

Taking into account that the associative algebra is generated by the finite set of elements $\left\{{u}_{j}\in A:j=\overline{1,m}\right\},$ it is easy to deduce from ${n}^{2}$ expansions of elements

${\text{a}}_{ij}:={c}_{k\left(i.j\right)}=\sum _{|{s}^{\left(1\right)}|\in {ℤ}_{+}}\sum _{{\sigma }_{1}\in {\Sigma }_{n}}{C}_{\left(k;{\sigma }_{1}\left(1\right),{\sigma }_{1}\left(2\right),...,{\sigma }_{1}\left(m\right)\right)}^{\left({s}_{1\text{\hspace{0.17em}}}^{\left(1\right)}{s}_{2}^{\left(1\right)}...{s}_{m}^{\left(1\right)}\right)}\left({u}_{{\sigma }_{1}\left(1\right)}^{{s}_{1}^{\left(1\right)}}{u}_{{\sigma }_{1}\left(2\right)}^{{s}_{2}^{\left(1\right)}}...{u}_{{\sigma }_{1}\left(m\right)}^{{s}_{m}^{\left(1\right)}}\right)+$
$+\sum _{|{s}^{\left(1\right)}|,|{s}^{\left(2\right)}|\in {ℤ}_{+}}\sum _{{\sigma }_{1},{\sigma }_{2}\in {\Sigma }_{n}}{C}_{\left(k;{\sigma }_{1}\left(1\right),{\sigma }_{1}\left(2\right),...,{\sigma }_{1}\left(m\right);{\sigma }_{2}\left(1\right),{\sigma }_{2}\left(2\right),...,{\sigma }_{2}\left(m\right)\right)}^{\left({s}_{1}^{\left(1\right)}{s}_{2}^{\left(1\right)}...{s}_{m}^{\left(1\right)};{s}_{1\text{\hspace{0.17em}}}^{\left(2\right)}{s}_{2}^{\left(2\right)}...{s}_{m}^{\left(2\right)}\right)}\left({u}_{{\sigma }_{1}\left(1\right)}^{{s}_{1}^{\left(1\right)}}{u}_{{\sigma }_{1}\left(2\right)}^{{s}_{2}^{\left(1\right)}}...{u}_{{\sigma }_{2}\left(m\right)}^{{s}_{m}^{\left(1\right)}}\right)×$

from A that the sum

iff ${c}_{k}=0$ for all $k=\overline{1,{n}^{2}}.$ Really, the sum of (3.5) under the $\pi$ -mapping can be now rewritten, respectively, as

with some D-coefficients from $\mathbb{K}$ for all $\text{\hspace{0.17em}}{\sigma }_{j}\in {S}_{n},$ depending quadratically on coefficients of expansions, staying at uniform and symmetric basis elements of the algebra A As the $\pi$ -mapping sends all of them, by definition, to zero, the resulting system (3.5) reduces to the set of algebraic equations

reducing successively for all ${\sigma }_{j}\in {S}_{n}$ to the condintions

being equivalent to the equalities ${c}_{k}=0$ for all $k=\overline{1,{n}^{2}}.$

As a simple consequence from Lemma 3.1 one derives the next proposition.

Proposition 3.2 The construted Lie algebra $\mathcal{G}$ is ad-invariant and $\pi$ -metrized.

Proof. Really, from the symmetry property (3.2) one easily obtains that

modulo $\pi$ -mapping for any elements a,b and $\text{c}\in \mathcal{G}.$ As the bilinear form (3.1 is non-degenerate, one has ${\mathcal{G}}^{\ast }\simeq \mathcal{G},$ that jointly with the ad-invariance property (3.9) means that the Lie algebra $\mathcal{G}$ is metrized.

Being interested in constructing integrable noncommutative dynamical systems on the algebra A we need to introduce into our analysis a “spectral” parameter $\lambda \in ℂ,$ responsible for the existence of infinite hierarchies of the corresponding dynamical systems invariants, guaranteeing their integrability. This wil be done in next Section, devoted to the Lie-algebraic analysis on loop-Lie-algebras, related with the Lie algebra $\mathcal{G},$ introduced above.

Consider now the Lie algebra $\left\{\mathcal{G},\left[\cdot ,\cdot \right]\right\},$ constructed above, and the related loop Lie algebra $\left\{\stackrel{˜}{\mathcal{G}}:=\mathcal{G}\otimes ℂ\left\{\left\{\lambda ,{\lambda }^{-1}\right\}\right\},\left[\cdot ,\cdot \right]\right\}$ of the corresponding $\mathcal{G}$ -valued Laurent series with respect to the parameter $\lambda \in ℂ,$

and define on it the corresponding to (3.1) modulo $\pi$ -mapping bilinear form $\left(\cdot |\cdot \right):\stackrel{˜}{\mathcal{G}}×\stackrel{˜}{\mathcal{G}}\to A:$

and define on it the corresponding to (3.1) modulo $\pi$ -mapping bilinear form

for any elements It is easy to observe that the bilinear form (3.11) is also symmetric and non-degenerate. Thus, the following proposition holds.

Proposition 3.3 The loop Lie algebra $\stackrel{˜}{\mathcal{G}}$ is ad-invariant and $\pi$ -metrized.

As the loop Lie algebra $\stackrel{˜}{\mathcal{G}}$ allows natural direct sum splitting $\stackrel{˜}{\mathcal{G}}{\stackrel{˜}{\mathcal{G}}}_{+}\oplus {\stackrel{˜}{\mathcal{G}}}_{-}$ into two Lie subalgebras ${\stackrel{˜}{\mathcal{G}}}_{+}$ and $\text{\hspace{0.17em}}{\stackrel{˜}{\mathcal{G}}}_{-},$ where

and

their adjoint spaces with respect to the bilinear form (3.11) split the adjoint loop space $\text{\hspace{0.17em}}{\stackrel{˜}{\mathcal{G}}}^{\ast }={\stackrel{˜}{\mathcal{G}}}_{+}^{\ast }\oplus {\stackrel{˜}{\mathcal{G}}}_{-}^{\ast }\text{\hspace{0.17em}}\text{\hspace{0.17em}}$ and satisfy the equivalences ${\stackrel{˜}{\mathcal{G}}}_{+}^{\ast }\simeq {\stackrel{˜}{\mathcal{G}}}_{-}$ and $\text{\hspace{0.17em}}{\stackrel{˜}{\mathcal{G}}}_{-}^{\ast }\simeq {\stackrel{˜}{\mathcal{G}}}_{+}.$

Let now a linear endomorphism $ℛ:\stackrel{˜}{\mathcal{G}}\to \stackrel{˜}{\mathcal{G}}$ equal $ℛ=$ $\left({P}_{+}-{P}_{-}\right)/2,$ where, by definitions, ${P}_{±}:\stackrel{˜}{\mathcal{G}}\to {\stackrel{˜}{\mathcal{G}}}_{±}\subset \stackrel{˜}{\mathcal{G}}$ are the projections on the corresponding subspaces ${\stackrel{˜}{\mathcal{G}}}_{±}\subset \stackrel{˜}{\mathcal{G}}.$ It is a well known property [14,15,32,33] that the deformed Lie product

for any satisfies the Jacobi condition and generates on the loop Lie algebra $\stackrel{˜}{\mathcal{G}}$ a new Lie algebra structure.

Within the classical Adler-Kostant-Symes Lie-algebraic approach, or its $ℛ$ -matrix structure generalization [14,15,32,33], the adjoint loop space ${\stackrel{˜}{\mathcal{G}}}^{\ast }$ is then endowed with the modified Lie-Poisson structure

for any basic functionals subject to which the whole set

of smooth Casimir functionals on ${\stackrel{˜}{\mathcal{G}}}^{\ast }$ is commutative with respect to the deformed Lie-Poisson structure (3.15) on ${\stackrel{˜}{\mathcal{G}}}^{\ast },$ that is ${\left\{\gamma ,\mu \right\}}_{♮}{=0}_{♮}\in {A}_{♮}\text{\hspace{0.17em}}$ for all $\gamma ,\mu \in I\left({\stackrel{˜}{\mathcal{G}}}^{\ast }\right)$ and, by definition, The latter makes it possible to construct integrable Hamiltonian flows on the associative algebra A as Poissonian flows on the co-adjoint orbits on the adjoint space ${\stackrel{˜}{\mathcal{G}}}^{\ast },$ generated by suitable loop Lie algebra $\stackrel{˜}{\mathcal{G}}$ Casimir gradient elements. Namely, if an element is fixed, the corresponding Hamiltonian flow on ${\stackrel{˜}{\mathcal{G}}}^{\ast }$ subject to the deformed Poisson bracket (3.15) and a Casimir funcrtional $\gamma \in I\left({\stackrel{˜}{\mathcal{G}}}^{\ast }\right)$ possesses the well known Lax type [33-40], representation

where $t\in \mathbb{K}$ is a related evolution parameter. The example of this construction and its Lie algebraic properties are discussed in the next Subsection.

##### Kontsevich type integrable systems on unital finitely generated free associative noncommutative algebras

Let a free unital finitely generated associative non-commutative algebra $A:=\mathbb{K}<{u}^{±},{v}^{±}>$ be the corresponding group algebra of a group $G\left\{u,v\right\},$ generated by two elements $u,v\in G.$ The algebra A is infinite dimensional with the countable basis ${L}_{A}<1,{u}^{j}{v}^{{s}_{1}-j},{v}^{j}{u}^{{s}_{1}-j},{u}^{j}{v}^{{s}_{2}-j}{u}^{j-k}{v}^{k-q},{v}^{j}{u}^{{s}_{2}-j}{v}^{j-k}{u}^{k-q},...:{s}_{1},{s}_{2},...\in ℤ>,\text{\hspace{0.17em}}$ the related two-dimensional matrix loop Lie algebra $\text{\hspace{0.17em}}\stackrel{˜}{\mathcal{G}}\mathcal{G}\otimes ℂ\left\{\left\{\lambda ,{\lambda }^{-1}\right\}\right\},$ $\mathcal{G}:=gl\left(2;A\right),$ is metrized subject to the bi-li near product (3.11) and generated by affine elements

with four basis Pauli matrix elements ${\sigma }_{k}\in gl\left(2;\mathbb{K}\right),k=\overline{0,3},$ and algebra components ${\text{a}}_{j}^{\left(k\right)}\in A,j\ll \infty ,k=\overline{0,3}.$ The corresponding Casimir functionals $\gamma \in I\left({\stackrel{˜}{\mathcal{G}}}^{\ast }\right)$ generate a Hamiltonian flow on points ${\stackrel{˜}{\mathcal{G}}}^{\ast }$ with respect to the Poisson bracket (3.15) in the Lax type form (3.17). To analyze this flow in detail, let us put, by definition, that the seed orbit point ${\stackrel{˜}{\mathcal{G}}}^{\ast }$ is given by the following $\lambda$ -squared expression

where $\left\{{\sigma }^{j}\in g{l}^{\ast }\left(2;\mathbb{K}\right):\text{tr}\left({\sigma }^{j}{\sigma }_{k}\right)={\delta }_{k}^{j},j,k=\overline{0,3}\right\}$ is the dual basis of the matrix space $g{l}^{\ast }\left(2;\mathbb{K}\right)\simeq gl\left(2;\mathbb{K}\right)$ and elements $\left\{{u}_{j}^{\left(k\right)}\in A:j=\overline{0,3},k=\overline{0,2}\right\}\text{\hspace{0.17em}}$ are coordinates of some A-algebra valued phase space ${M}_{A}^{\left(0|2\right)}$ in a general position. In particular, we will choose the following dual bases:

in $gl\left(2;\mathbb{K}\right)$ and

${\sigma }^{0}=\left(\begin{array}{cc}1/2& 0\\ 0& 1/2\end{array}\right),{\sigma }^{1}=\left(\begin{array}{cc}0& 1\\ 0& 0\end{array}\right),{\sigma }^{2}=\left(\begin{array}{cc}0& 0\\ 1& 0\end{array}\right),{\sigma }^{3}=\left(\begin{array}{cc}1/2& 0\\ 0& -1/2\end{array}\right)$

in $gl{\left(2;\mathbb{K}\right)}^{\ast }.$ Moreover, we also will assume that A-algebra valued coefficients of the phase space ${M}_{A}^{\left(0|2\right)}$ in (4.2) are representable subject to the basis of A as

following the result obtained in [31].

As a first important task, we will calculate the corresponding Poisson structure on the related A-algebra valued phase space generated by coefficients, presented in the expression (4.4). To do this, we need to take into account that the phase space being endowed with the $ℛ$ -modified Poisson structure (3.15), is strongly reduced via the Dirac scheme [4,32], subject to the set

${\phi }_{3}={u}_{2}^{\left(0\right)}=0,{\phi }_{4}={u}_{3}^{\left(2\right)}=0,{\phi }_{5}={u}_{3}^{\left(0\right)}+1=0\right\}$

of algebraic constraints, imposed on the phase space ${M}_{A}^{\left(0|2\right)}.$ The latter means that the true Poisson structure on the reduced phase space coincides with the corresponding Dirac type reduction of the $ℛ$ -modified Poisson structure, defined on the full phase space $\text{\hspace{0.17em}}{M}_{A}^{\left(0|2\right)}.$ As a result of simple enough yet cumbersome calculations we arrive at the following Poisson brackets

on the reduced phase space

Having taken as a Hamiltonian operator one easily obtains the following [5], nonlinear integrable Kontsevich dynamical system

on the reduced phase space $A=\mathbb{K}〈{u}^{±},{v}^{±}〉.$ Moreover, owing to the Lax type representation (3.15), the Kontsevich dynamical system (4.7) proves to be equivalent to the following matrix commutator equation

for any $\lambda \in \mathbb{K}$ in the Lie algebra $\stackrel{˜}{\mathcal{G}},$ where the A-valued matrix

$\begin{array}{l}={\sigma }_{0}\left({v}^{-1}-v+u+1\right)/2+{\sigma }_{1}\lambda v+\\ {\sigma }_{2}{v}^{-1}+{\sigma }_{3}\left({v}^{-1}-v+u-1\right)/2\in \stackrel{˜}{\mathcal{G}}\text{\hspace{0.17em}}.\end{array}$

Taking as Hamiltonian functions the algebraic expressions one can obtain a complete set of $\pi$ -commuting to each other conservation laws of the Kontsevich dynamical system (4.7), thus proving its generalized integrability. Moreover, choosing both another group algebra and orbit elements ${\stackrel{˜}{\mathcal{G}}}^{\ast },$ one can construct the same way many other integrable Hamiltonian systems on the associative noncommutative phase space A, that is planned to be a topic of a next investigation.

### Conclusion

In this work we succeeded in revisting the classical Poisson manifolds approach to Hamiltonian operators on functional noncommutative manifolds, as well as presented it simple and natural realization, generated by associative noncommutative group algebra. The latter appeared to be very useful for describing a wide class of new Lax type integrable nonlinear Hamiltonian systems on associative noncommutative algebras, interesting for diverse applications in modern quantum physics.

The authors are cordially indebted to Prof. Anatol Odziewicz for fruitful and instructive discussions during the XXXVIII Workshop on Geometric Methods in Physics held on Juny 30 - July 06, 2019 in Bialowieza, Poland. A.P. thanks also the Departments of Mathematical Sciences of the Rutgers University and the NJIT University of Technology (NJ, USA) for invitations to visit them during the Spring Semester-2019, where there was prepared an essential part of the present work. The aknowledgements belong to the Department of Physics, Mathematics and Computer Science of the Cracov University of Technology for a local research grant F-2/370/2018/DS.

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