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\begin{titlepage}

\noindent
% {\bf H-UM \& JS: version of \today} \\[.3em] 
Submitted to the 30th International Conference on 
High-Energy Physics ICHEP2000, \\ 
Osaka, Japan, July 2000


\vspace*{3cm}

\begin{center}
  \Large
  {\bf 
Search for QCD Instanton Induced Events in Deep-Inelastic Scattering at HERA
 }
  \vspace*{1cm} \\
  {\Large H1 Collaboration} 
\end{center}

\begin{abstract}
\noindent
Signals of QCD instanton induced processes are searched for
in deep-inelastic scattering (DIS) at HERA
in a kinematic region defined by the Bjorken-scaling variables 
$x > 10^{-3}$, $0.1 < y < 0.6$ and the polar angle of the
scattered positron $\theta_{el} > 156^o$. 
The cross section for QCD instanton induced processes
in this domain is predicted to be sizeable, but 
two to three orders of magnitude
below the standard DIS cross section.
%
Several observables characterising hadronic final state 
properties of QCD instanton induced events are used to
discriminate them from the standard DIS background
and to identify a possibly instanton enriched domain.
%
%With the help of a Monte Carlo simulation for the QCD instanton process
%and the standard DIS a phase region is identified 
%using a simple cut technique 
%where only about $0.1 \%$ of the DIS background is left, but $10 \%$
%of the instanton induced events remain. In this region
%more events are found in the data than predicted by the 
%standard QCD models.
%The shape of three observables used to identify the 
%instanton enriched region
%is qualitatively similar to the expected instanton signal.
%Its size is still small compared to the DIS background 
%and is at the level of the difference of two different QCD models. 
%Furthermore, the shape of some of the three other
%discriminating observables is not well reproduced by the standard
%QCD models and does not particularly favour an interpretation of
%the data in terms of instanton induce processes 
%in the present implementation in the QCD instanton Monte Carlo generator.
%
In a phase space region where a reduction of the
standard DIS background to the percent
level is achieved according to Monte Carlo models,
more events are found in the data than expected by standard 
DIS models.
The size of the excess is at a level comparable to the difference
of the QCD-based standard DIS models, but is - for the
discriminating observables - qualitatively similar to the
expected instanton signal.
For other discriminating observables the data do not
particularly favour an interpretation of the excess in terms
of instanton induced processes as modelled in the 
current implementation of the QCD instanton Monte Carlo
simulation.
%
%For various values of the kinematic \xprime and \qprimesq variables
%characterising the hard instanton subprocess an upper limit
%is derived. 
Upper limits on the QCD instanton production cross section 
between $100$ \pb and $1000$ \pb are derived only from the expected
instanton hadronic final state topology and the number of observed
events in the data.
They exclude the steep rise of the instanton cross
section towards large instanton sizes
as would be obtained from a naive extrapolation of 
instanton perturbation theory. The absense of this steep
rise is in agreement 
with comparisons of perturbative calculations to lattice simulations.
%
%In the region where I-theory is expected to be valid,
%the upper limit is about one order of magnitude above
%the prediction.
%
%Further studies on the influence of the theoretical uncertainties
%of the expected instanton signal and a better understanding of
%the standard QCD background processes are needed. 
%
%Assuming that the hadronic final state of instanton-induced processes is
%correctly simulated by QCDINS, an upper limit on the cross section
%is derived of $XXX$ \pb is derived.
%The data exclude that not more than $XXX \%$ of the DIS events are induced
%by instantons as simulated by the QCDINS program.

\end{abstract}


\vfill
\begin{flushleft}
  {\bf Abstract: 972 } \\
  {\bf Parallel session: 3} \\
  {\bf Plenary talk: 11 } 
\end{flushleft}

\end{titlepage}

\pagestyle{plain}

\section{Introduction}
The Standard Model is known to contain certain hard processes which cannot be 
described by perturbation theory. These violate the 
classical laws of baryon and lepton number conservation
in case of the electroweak and chirality conservation in case of
the strong interaction \cite{inst:thoofta,inst:thooftb,inst:thooftc}, respectively. 
Such anomalous processes are induced by instantons \cite{inst:belavin}.
QCD instantons  are non-perturbative fluctuations of the gluon field 
inducing hard processes and represent tunnelling transitions between 
topologically inequivalent vacua.
%
%In the deep-inelastic scattering (DIS) regime 
%the quark $q'$,
%originating from a photon splitting into a $q\bar{q}$ pair in
%the instanton background (see Fig.~\ref{kin-var}), provides  
%a generic hard scale naturally limits
%the instanton size $\rho$ and makes a quantitative prediction of the
%cross-section using instanton perturbation theory
%possible~\cite{inst:balitsky1,inst:moch,inst:RS4}.
%
Deep-inelastic scattering (DIS) offers a unique 
opportunity~\cite{inst:vladimir} to discover processes
induced by QCD instantons through a sizeable rate,
calculable\footnote{For an exploratory calculation of the
instanton contribution to the gluon structure function at 
large $x_g > 0.3-0.35$, see ref.~\cite{inst:balitsky1}.}
within ``instanton-perturbation theory''
\cite{inst:moch,inst:RS4,inst:rs-lat}, along with a characteristic
final state signature \cite{inst:vladimir,inst:greenshaw,inst:mcws99}.
For a recent review, see ref.\cite{inst:ringberg00}.

At HERA, colliding $27.5$\GeV positrons on $820$\GeV protons, 
the size of the predicted cross section is large enough     
to make an experimental observation possible.
The expected signal is, however, still small compared to the
standard DIS process. 
The suppression of the standard DIS background
is therefore the key issue in this analysis.
%
QCD instanton-induced processes (I-processes) can be discriminated
from standard DIS by their 
characteristic hadronic final state signature 
consisting of a large number of hadrons at high transverse energy
emerging from a ``fire-ball''-like topology  
\cite{inst:vladimir,inst:greenshaw,inst:mcws99,inst:ringberg00}.

Limits on I-processes based on existing hadronic final state
DIS data have already been derived in ~\cite{h1:k0, h1:mult,carlikuhlen}. 
Here, we present for the first time a dedicated search
for I-processes at HERA.
The data corresponding to an integrated luminosity of $15.8$ {\rm pb}$^{-1}$
were collected in the year $1997$.
We cover the kinematic region defined
by the Bjorken-scaling variables 
$x > 10^{-3}$, $0.1 < y < 0.6$ and the polar angle of the
scattered electron $\theta_{el} > 156^o$.

\section{Production of QCD Instanton-induced Processes at HERA}
\label{sec:qcdtheo}
Instanton induced processes in DIS are dominantly produced in a photon gluon 
fusion process as sketched in Fig.~\ref{kin-var}. 
Within the framework of A. Ringwald and F. Schrempp
\cite{inst:vladimir,inst:moch,
inst:RS4,inst:rs-lat,inst:mcws99,inst:ringberg00} 
the instanton induced event signature may be described
by the following basic reaction:
\begin{equation}
\gamma^* + g \to \sum_{n_{\rm flavours}} (\bar{q}_R + q_R) + \, n_g \, g,
\end{equation}
where $q_R$ ($\bar{q}_R$) denotes right handed quarks \footnote{
Right handed quarks are produced in instanton processes.
Left-handed quarks are produced in anti-instanton processes. 
The hadronic final state 
referring to  instantons and anti-instantons respectively,
can only be distinguished by the
chirality of the quarks. Both processes enter in the cross section.}
and $g$ gluons.
A photon splitting into a quark-anti-quark pair
in the background of an instanton or an anti-instanton fuses with
a gluon from the proton. 
Besides the current-quark ($q^{\prime\prime}$), the partonic final state 
consists of $2 n_f - 1$  right-handed
(massless) quarks and anti-quarks. 
In every I-induced event, one quark anti-quark pair 
of all $n_f(=3)$ flavours is simultaneously 
produced~\footnote{If kinematically possible, charm and bottom quarks
can also be produced. The estimation of the cross section is, however,
difficult and is not considered here.}.
In addition, a mean of 
$\langle n_g \rangle ^{(I)} \sim {\cal O}(1/\alpha_s)  \sim  3$
gluons are emitted in the I-process.
%
%
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
\begin{figure}[h]
   \centering
\hspace{1.0cm}
\begin{tabular}{ll}
\mbox{
 \epsfig{file=H1prelim-00-025.fig1.eps,width=7.cm,}
% bbllx=80pt,bblly=355pt,bburx=410pt,bbury=600,clip=}
}
&
\begin{tabular}{l}
 \vspace{-5.5cm} \\
 DIS variables: \\
   $S=(e+P)^2$\\
   $\Qsq = - q^2 = -(e-e')^2$ \\
   $ x = \Qsq / \; (2 P \cdot q) $ \\
   $ W^2 =(q+P)^2 = \Qsq (1 - x)/x$ \\
   $ \hat{s} = (q+g)^2$ \\
   $ \xi = x \;(1+\hat{s}/Q^2)$ \\ \\
 Variables of I-subprocess: \\
 $\qprimesq=- {q'}^2 = - (q-q'')^2 $ \\
 $x'= \qprimesq / \;(2 \; g \cdot q' ) $ \\
 $W_I^2= (q'+g)^2 = \qprimesq ( 1 - \xprime )/ \xprime $\\
\end{tabular}
\end{tabular}
%}
\vspace{0.3cm}
   \caption[Kinematic variables of QCD instanton induced process
     in deep-inelastic scattering]
     {Kinematic variables of the dominant instanton induced process
      in deep-inelastic scattering. 
      The virtual photon $\gamma$ 
      (4-momentum $q=e-e'$), emitted by the incoming electron $e$,
      fuses with a gluon ($4$-momentum $g$) of the proton
      (4-momentum $P$).
      The gluon carries a fraction $\xi$ of the (longitudinal) 
      proton 4-momentum. The virtual quark entering the 
      instanton subprocess has $4$-momentum $q'$,
      while the outgoing quark ({\it = current quark}) from the 
      $\gamma \rightarrow q \ol q $-process
      has $q^{\prime\prime}$. $x'$ is defined in analogy
      with $x$, but cannot be illustrated in a simple way.
      $0 \leq x \leq x /\xi \leq x' \leq 1$ holds. 
      $W_I$ is the invariant mass of the quark gluon ($q'g$) system
      and $W$ is the invariant mass of the total hadronic system 
      (the $\gamma P$ system).
      $\hat{s}$ is the invariant mass squared of the $\gamma g$ system.}
   \label{kin-var}
\end{figure}
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
%
These partons emerge isotropically distributed from the I-process.
One expects therefore a
pseudo-rapidity~\footnote{The pseudo-rapidity of a 
particle is defined as $\eta \equiv - \ln ( \tan \theta / 2 )$ where $\theta$ is 
the polar angle with respect to the proton direction.}  ($\eta$)
region (with a width of $\approx 1.1 \; \eta$ units)
densely populated with particles at high transverse momentum
which are homogeneously distributed in azimuth. 
%The width of this ``instanton-band'' has been estimated to
%$\simeq \pm 1.1$ rapidity units.  
Besides this pseudo-rapidity band, 
the hadronic final state of I-induced events 
exhibits a current jet emerging from
the outgoing current quark.
%
The high density of partons emitted in the I-process leads
to a high mean multiplicity of charged particles in every event.
Moreover, since all (effectively massless) flavours are produced
in any event, 
more mesons containing strange quarks should be found in 
I-induced events than in normal DIS events. 

The actual number of produced hadrons and their energy
crucially depends on the squared centre of mass energy 
$W_I^2 = {(q^\prime + \xi p)}^2$ available 
in the I-system. $W_I^2 = \qprimesq (1 - \xprime)/\xprime$ 
is closely connected to the variables \qprimesq and \xprime
describing the kinematics of the I-subprocess. 
These variables are analogous to the Bjorken scaling 
variables $x$ and $Q^2$.
The knowledge of the distribution of these variables
is therefore indispensable for the correct prediction
of the hadronic final state.
Since the I-cross section can been calculated
for large \qprimesq and \xprime this distribution is known
within I-perturbation theory \cite{inst:RS4}.
Towards low values, however, the I-cross section is steeply
increasing. In this region the approximations made to derive
the cross section in I-perturbation theory no longer valid.
The fiducial region where I-perturbation theory is expected
to work has been estimated from a high quality lattice
simulation of crucial quantities entering in the instanton
calculations \cite{inst:rs-lat}.
%where the
%instanton density has been directly calculated using lattice
%simulations 

For the fiducial region, $\xprime > 0.35$, $\qprimesq > 113$ \GeVsqx,
$x > 10^{-3}$ and $0.1 < y < 0.9$, an update of the published
I-cross section \cite{inst:RS4}, referring to the 1998 world
average of the strong coupling constant \cite{pdg98}, 
has been given in \cite{inst:ringberg00,inst:schremppdis00} to be:
%\begin{equation}
$
\sigma_{ins} = 89_{-15}^{+18} \; {\rm pb}.
$
%\end{equation}
To further reduce remaining theoretical uncertainties,
ideally, an additional cut, $Q^2 > 113 \GeVsqx$, has to be applied.
In this domain the cross section is:
%\begin{equation}
$
\sigma_{ins} = 29_{-7.5}^{+10} \; {\rm pb}.
$
%\end{equation}
%
The quoted error only contains the uncertainties of $\sigma_{ins}$ 
obtained from varying the strong coupling constant within the
error of the world average. 
This cross section has been derived for three-flavours. 
The calculation is based
on a two loop renormalisation group invariant expression of the
instanton density. 
%significantly reduces the residual renormalisation
%scale dependence of the instanton subprocess cross-section.

While this prediction has not yet reached the same quantitative
level as current standard perturbative QCD calculations, 
the cross section is large enough to make
dedicated searches for instanton induced processes interesting. 

\section{QCD Monte Carlo Models}
\subsection{Standard DIS Monte Carlo Models}
A simulation of the detailed properties of the hadronic
final state in DIS is available in the form of QCD Monte Carlo
event generators. These include the matrix
element of the hard subprocess to first order in the
strong coupling constant $\alpha_s$, approximations of
higher order QCD radiation effects, and a model to describe the
non-perturbative transition from partons to hadrons.


The RAPGAP Monte Carlo~\cite{rapgap} incorporates the
${\cal O} (\alpha_s)$ QCD matrix element and models higher order parton emissions
approximately to all orders $\alpha_s$ using the concept of parton showers~\cite{shower} 
based on the leading logarithm DGLAP equations~\cite{dglap}.
QCD radiation can occur before and after the hard subprocess. 
The formation of hadrons is performed using the LUND string model~\cite{lund} 
implemented in JETSET~\cite{jetset}. 
This QCD Monte Carlo is called ``MEPS'' in the following.

A completely different treatment of the perturbative phase is implemented
in ARIADNE~\cite{ariadne}, where
gluon emissions are simulated using the colour dipole model (CDM)~\cite{cdm}
assuming a chain of independently radiating
dipoles spanned by colour connected partons. No distinction between
initial and final state partons is made.
The first emission in the cascade is corrected to reproduce the matrix element to first 
order $\alpha_s$~\cite{ariadneme}. 
The hadronisation is performed using JETSET.
This QCD Monte Carlo is called ``CDM'' in the following.

The program HERACLES~\cite{heracles} is interfaced to ARIADNE and RAPGAP to include
${\cal O}(\alpha)$ electroweak corrections to the lepton vertex.

The PHOJET~\cite{phojet} Monte Carlo program is used to calculate the photoproduction
background. It contains the first order matrix elements for direct and
resolved processes, parton showers
and a phenomenological description of soft processes.

Both Monte Carlo DIS samples have been generated with the
CTEQ4M~\cite{cteq4} parton density function and are reweighted using a
parametrisation of the $96/97$ proton structure function
as measured in a recent H1 analysis.

All above the standard DIS Monte Carlo generators
are based on leading order calculations.
The correct QCD dynamics, in particular in the small-$x$ regime,
is still under debate at HERA.
The MEPS and the CDM models have been comprehensively compared to a variety of
hadronic final state data and an attempt has been made to optimise
free model parameters \cite{inst:mcws99tuning}.
No parameter set was found that describes the whole range
of distributions over the full studied kinematic domain $5 \lsim \Qsq \lsim 5000$ \GeVsqx.
It is therefore questionable to what extent 
the currently available QCD models
can give a fair
representation of the standard DIS hadronic final state.
In this analysis the Monte Carlo models have been used with their default values. 

\subsection{QCD Instanton Monte Carlo Model} 
QCDINS~\cite{inst:schremppdis95,inst:qcdins} is a 
Monte Carlo package for simulating 
QCD-instanton induced scattering processes in DIS.
It acts as a hard process generator embedded in the HERWIG~\cite{herwig}
program.
The hard process is treated according to the physics assumptions
explained in section \ref{sec:qcdtheo}.
We use the default values of the QCDINS 2.0 version, i.e.
$\xprime > 0.35$, $\qprimesq > 113$ \GeVsq and $n_f=3$.
The CTEQ4L~\cite{cteq4} parton density function is used.
After assembling the hard  I-subprocess, further gluon emissions
are simulated in the leading-logarithm approximation. The coherent
branching algorithm implemented in HERWIG is used.
The transition from partons to the observable hadrons is performed
with the cluster fragmentation model \cite{inst:cluster}, where
the primary hadrons are produced from mainly 
isotropic two-body decays of 
colour-singlet parton clusters. As an alternative the LUND
string model can be also be used.
QED radiation is not implemented.

%Little experience is available 
It is not clear whether the currently used hadronisation
models implemented in HEP event simulation programs
are appropriate to describe the fragmentation
of the large number of ${\cal O}(10)$ partons produced 
by the I-process in a narrow pseudo-rapidity region with high transverse energy.
%
However, the observables studied are mainly influenced by the hard 
instanton-subprocess and depend only slightly on the 
hadronisation model~\cite{inst:mcws99}. 
This has been studied by using JETSET
instead of the cluster fragmentation model and by changing
free parameters in the hadronisation models.

\newpage
\section{The H1 Detector }\label{detector}
% **********************************************************************
A detailed description of the H1 detector can be found elsewhere~\cite{H1det}.
Here we briefly introduce the detector components most relevant 
for this analysis: The liquid argon (LAr) calorimeter,
the backward lead-fibre calorimeter (SpaCal) 
and the tracking chamber system.

The LAr calorimeter~\cite{h1lar} 
consists of an electromagnetic section ($20-30$ radiation lengths) 
with lead absorber and a hadronic section with steel absorber.
The total depth of both calorimeters 
varies between $4.5$ and $8$ interaction lengths. 
The hadronic energy flow is mainly measured by the
LAr calorimeter extending over the polar angle range
$4^\circ < \theta <  154^\circ$ with full azimuthal coverage.
%\footnote{The polar angle $\theta$ is defined with respect to the proton
%beam direction ($+z$ axis).}. 
Electromagnetic shower energies are measured with a resolution
of $\sigma_E/E \approx 0.12/\sqrt{E \;[\GeV]} \oplus 1 \% $~\cite{electrons}.
Test beam measurements of the LAr~calorimeter modules show an
energy resolution of 
$\sigma_{E}/E\approx 0.50/\sqrt{E\;[\GeV]} \oplus 0.02$  
after software weighting for charged pions~\cite{pions}.

The backward lead-fibre calorimeter SpaCal~\cite{h1SpaCal}
covers the polar angle range $153^\circ < \theta <  177^\circ$. 
In the electromagnetic section, with  a depth of $28$ radiation lengths,  
electrons are measured with an energy resolution of 
$\sigma_E/E \approx 0.025/\sqrt{E \;[\GeV]} \oplus 2.5 \%$.
In addition the SpaCal has a hadronic section of two interaction
lengths to measure hadrons. 

The calorimeters are 
surrounded by a superconducting solenoid providing a uniform
magnetic field of $1.15$ {\rm T} parallel to the beam axis in the tracking region.

Charged particle tracks are measured in two concentric jet drift chamber 
modules (CJC), covering the polar angle range  
$ 15^\circ < \theta < 165^\circ$~\cite{cjc}.
%The forward tracking detector covers $7^\circ < \theta < 25^\circ $ 
%and consists of drift chambers with alternating planes 
%of parallel wires and others with wires in the radial direction
%~\cite{fwdtracker}.
A backward drift chamber BDC %~\cite{bdc} 
%with an angular acceptance of $???^\circ < \theta < ???^\circ$
aids identification of positrons scattered into the SpaCal calorimeter.

The luminosity is measured using the elastic Bethe-Heitler
process. % with an accuracy of $1.5 \%$. %~\cite{lumi}. 
The final state positron
and photon are detected in calorimeters situated close to the
beam pipe at distances of $33$ {\rm m} and $103$ {\rm m} from the interaction
point in the positron beam direction.
%
\section{DIS Event Selection}

The data used in this analysis were collected in the year
$1997$ with the H1 detector at the $ep$ collider HERA.
During this time HERA collided positrons at an energy
of $E_e = 27.5$~\GeV with protons at an energy of 
$E_p = 820$~\GeVx.
The accumulated data sample corresponds
to an integrated luminosity of about $15.8$~{\rm pb}$^{-1}$.

The scattered positron is identified as the electromagnetic energy
deposition with the highest energy in the SpaCal calorimeter.
It is required to lie well within the calorimeter and trigger acceptance
of polar angles between $156^\circ$ and $176^\circ$.
A minimal positron energy of $E^\prime_e \ge 10$~\GeV~ is required.
To suppress background from misidentified photoproduction events
the distance to the closest signal in the preceding drift chamber
(BDC) has to be smaller than $3$~{\rm cm}.
The events are triggered by demanding a localised
energy deposition in the SpaCal together with loose track requirements in the
multi-wire proportional and the drift chambers.

Furthermore $35\,\GeV < \sum (E - p_z) < 70\,\GeVx$,
where the sum runs over all objects belonging to the
hadronic final state (see section \ref{sec:obs}), is required.
The position of the  $z$ coordinate of the reconstructed 
event vertex must be 
within $\pm 30\,\mbox{\rm cm}$ of the nominal interaction point.

The photon virtuality $Q^2$ and the Bjorken scaling variable $x$
are reconstructed from the scattered positron. The analysis
is performed in the phase space region defined by
$\theta_{el} > 156^o$, $ 0.1 < y < 0.6$ and $x >10^{-3}$, where
$\theta_{el}$ is the polar angle of the scattered positron.

The DIS data sample consists of $275000$ events.
The simulated events reproduce the distributions in 
energy and angle of the scattered positron 
as well as the kinematic variables $x$, $Q^2$ and $y$ 
to the $3\%$ level.
% 
%For $0.1 < y < 0.35$ a difference
%of the Monte Carlo and the data of less then $1\%$ is found.
%Only at high $y$ the Monte Carlo falls below the data
%by about $5\%$. This is the region where possible contributions
%from misidentified photoproduction processes are largest.
%It can therefore be concluded that the photoproduction
%background in the total inclusive DIS sample is much smaller
%than $5\%$. This is also in agreement with a Monte Carlo simulation based on PHOJET.
The contamination by events with misidentified positrons
stemming from $\gamma p$ reactions is below
$2 \%$ and is neglected in the following. 
This was estimated using the Monte Carlo
simulation program PHOJET~\cite{phojet}.

\section{Definition of the Discriminating Observables} \label{sec:obs}
The observables used to discriminate I-induced events from
standard deep-inelastic scattering are based on the hadronic
final state. For most of the observables the energy flow
in the detector is reconstructed by combining the
calorimetric energy depositions in the LAr and the SpaCal
calorimeters  and the momenta of low momentum tracks ($p_t < 2$~\GeVx) 
in the central jet chamber according to the procedure described in ~\cite{h1highq2}.
Charged particles with transverse momenta of $p_t > 0.15$ \GeV
are identified within the acceptance of
the central jet chamber ($20^o < \theta < 155^o$).
%Since in $1997$ certain sectors of the CJC had an efficiency
%decreasing in time and since the efficiency drop is not
%perfectly simulated by the Monte Carlo, tracks in the
%region of $-160  < \phi < -80$ do not enter in the
%definition of $n_B$ in both data and Monte Carlo. 
The hadronic final state objects are boosted to the hadronic
centre-of-mass (hcms) frame\footnote{The hcms is defined by
$\vec{q} + \vec{p} = 0$, where $\vec{q}$ ($\vec{p}$) is the $4$-momentum
of the photon (proton).}.
 
Jets are defined by the cone algorithm \cite{pozo,cdfcone} 
with a cone radius of $R = \sqrt{\eta^2 + \phi^2} = 0.5$. 
The jet with the highest transverse energy (\etjetx)
is used to estimate the $4$-momentum $q^{''}$ of the current quark
(see Fig.~\ref{kin-var}).
Once the current jet is found, \qprimesq can be reconstructed
from the particles associated to the current jet 
and the photon reconstructed using the momentum of the scattered positrons.
We treat \qprimesqrec as a good discriminating observable.
Due to the limited accuracy of the \qprimesq reconstruction, 
\qprimesqrec can not be used to experimentally control the ``true'' \qprimesq 
region of the I-processes.  
The achieved \qprimesq resolution is about $20 - 30 \%$.
However, the distribution of the true over the reconstructed value
exhibits large tails. The relatively small cone radius of $R=0.5$
gives the best result. More information on the \qprimesq reconstruction 
can be found in \cite{inst:mcws99,inst:jgerigk}. 
The reconstruction of the variable \xprime is very difficult\footnote{ 
Due to the inherent difficulties to  reconstruct \xprime
experimentally, 
the data used for the present analysis do not
incorporate a cut on \xprimex, necessary to warrant the validity of
I-perturbation theory. As noticed in Ref. \cite{inst:rs-lat},  this 
presumably does not prevent a comparison with the
Ringwald-Schrempp predictions for the following reason. 
The lattice data for the $I\overline{I}$-distance 
distribution (from which the minimal theoretical \xprimex-cut was
deduced  \cite{inst:rs-lat}) happen to exhibit an extremely rapid
suppression of I-effects for small $I\overline{I}$-separation, corresponding to
$\xprime < 0.35$. Therefore, I-contributions to the data from  this $\xprime$
region outside the validity of I-perturbation theory are probably also small.}. 



The objects belonging to the jet are not used in the following observables.
The $E_t$-weighted rapidity mean $\bar{\eta}= \sum_h E_{t,h} \; \eta_h / \sum E_{t,h}$ 
of all remaining objects
is used as an estimator of the position of the instanton band,
which is defined by ~$\bar{\eta} \pm 1.1$.
Within this rapidity region the number of charged particles (\nbx)
is counted and the total scalar transverse energy (\etbx) is measured. 
Furthermore, the axis $\vec{i}$ is found for which the summed projections of the
$4$-momenta of all hadronic objects are minimal resp. 
maximal \cite{inst:greenshaw}.
The relative difference between $E_{in}= \min_i{\sum_h |\vec{p}_h \cdot \vec{i} |}$
and $E_{out}= \max_i{\sum_h |\vec{p}_h \cdot \vec{i} |}$ is called
$\deltabx = (E_{in}-E_{out})/E_{in}$.
This quantity measures the $E_t$ weighted azimuthal isotropy of an event.
For isotropic events $\Delta_b$ is expected to take small
values while for pencil-like events $\Delta_b$ should be large.

%
The vectorial sum of all measured final state objects
not associated to the ``current'' jet (see above)
is used to perform a boost to their rest system defined by
$\sum_h \vec{p}_h = 0$. In this system, which is an approximation
to the instanton rest system defined by: $\vec{q'}+\vec{g}=0$ 
(see Fig.\ref{kin-var}), the sphericity \sph is calculated.
%
%The sphericity is defined as 
%$\min{ 3/2 \; (\sum_h p_{t,h} \; \vec{i}} \ \sum_h \vec{p}_h^{\; 2})$,
%where $\vec{i}$ is an arbitrary axis with respect to which the transverse
%momentum  $P_t$ is calculated.
%


\section{Search Strategy and Results} 
\subsection{Description of the Observables in the Inclusive DIS Sample} 
The search strategy is based on three of the six observables
presented in section \ref{sec:obs}:
the multiplicity in the band ($n_b$),  
the sphericity as calculated in the rest system of all
final state objects not associated to the current jet (\sphx) and
the reconstructed \qprimesqrecx.
These observables will be exploited to define an possibly
instanton enriched data sample.


The distributions of the discriminating observables for data, for the standard DIS
Monte Carlo simulation and for the I-process
are shown in Fig.~\ref{fig:datamclin} and Fig.~\ref{fig:datamclog}.
They are all fairly well described by the standard DIS Monte 
Carlo simulations.
Both standard DIS models overshoot the data for $1 < \nb < 5$
and undershoot the data for $5 < \nb < 10$ by $5 - 10 \%$.
For the highest charged particle multiplicities
discrepancies up to $20 \%$ are found.
For sphericity values between $0.1 < \sph < 0.4$ the standard DIS
Monte Carlo models predict $5 - 10 \%$ more events than
found in the data, while for $\sph > 0.4$ $5 - 20 \%$
less events than in the data are predicted.
For values below $100$ \GeVsq the \qprimesqrec distribution is 
described within $5 \%$, for higher values differences of
up to $10 \%$ are found.

The three other observables not used to define the 
instanton-enriched data sample, i.e.
\etjetx, \etb and \deltabx, contain additional information.
% about the physical origin 
%of the remaining events after the cuts on the three other
%previously discussed observables.
They are shown in Fig.~\ref{fig:datamclinother} and Fig.~\ref{fig:datamclogother}.
The \deltab distribution is fairly well described (within $10 \%$) 
by both standard DIS simulations.
For the \etjet the two standard DIS Monte Carlos simulations behave differently.
MEPS is about $10 \%$ below (above) the data for
$\etjet < 2.5$ \GeV ($\etjet > 2.5$ \GeV). In the tail of this
distribution the data are well reproduced up to the largest 
accessible values.
CDM describes the data within $5 \%$ for $\etjet \lsim 7.5$ \GeVx,
but then exhibits an increasingly too hard \etjet spectrum
toward larger \etjetx. However, for \etjet ranges where an I-signal is
expected, the difference between the data and the CDM simulation is not
bigger than $20 \%$.
%
A harder tail than found in the data is also seen in the \etb
distribution. Again the MEPS simulation gives a good description
in this domain ($\etb > 10 \GeVx$). 
The hard transverse energy tail produced by CDM has also been
observed in dijet production \cite{h1vancouver}. It can be brought
in agreement with the data
by adjusting free model parameters \cite{inst:mcws99tuning}.
%For low \etb values the data are up to $20 \%$ higher 
%than both Monte Carlo simulations and also disagree with each other. 
For $2 < \etb < 10 \GeV$ deviations between the data and the standard
DIS models within $10\%$ are seen. The data are, however, always in between
the standard DIS simulations. At very low \etb values ($\etb < 2 \GeV$)
the data exceed the simulations by $20 \%$.
%

The instanton prediction is shown as a solid line 
in Fig.\ref{fig:datamclinother}.
One can see that the expected instanton signal is about two to three
orders of magnitude smaller than the standard DIS background.
Therefore additional cuts are needed to enhance the signal
over the background.

\subsection{Search Strategy Based on Simple Cuts}
\label{sec:strategy} 
The strategy to reduce the standard DIS background 
is based on the three observables shown in Fig.~\ref{fig:instmc}.
The shape of these observable is different for I-processes and standard
DIS.
To find the optimal cut scenario $125$ combinations of $5$ different
values of the three
observables are investigated using simulations of the standard DIS background 
and of the I-signal. 
The following cuts are applied:
$
\nb > 5, 6, 7, 8, 9
$ ;
$
\sph > 0.4, 0.5, 0.55, 0.6, 0.65  
$ ;
$
95, 100, 105, 110, 115 <  \qprimesqrec < 200 \GeVsqx
$. 
From 125 cut combinations   
three scenarios are chosen according to the following criteria: \\
(A) The highest instanton efficiency ($\epsilon_{ins}$) \\ % $\approx 30 \%$) 
(B) High $\epsilon_{ins}$ at reasonable background reduction ($\epsilon_{dis}$) \\
(C) Highest separation power ($\epsilon_{ins}/\epsilon_{dis}$)
     %$\approx 0.13-0.16 \%$)
at  $\epsilon_{ins}$ $\approx 10 \%$.\\

The cut values, the instanton efficiency $\epsilon_{ins}$ and the
standard DIS efficiency $\epsilon_{dis}$ for each chosen 
cut combination are summarised in table \ref{table:cuts}.
A background reduction to the permille level is achieved while
a sizeable instanton efficiency is ensured.
A maximal separation power $\epsilon_{ins}/\epsilon_{dis}$ of $86$ is reached.


\subsection{Experimental Results}


%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
\begin{table}[t]
\begin{center}
\footnotesize
\begin{tabular}{c|ccc}
    & CUT A & CUT B & CUT C \\
\hline
\nb &  $\nb \ge 5$ & $\nb \ge 7$ & $\nb \ge 8$ \\
\qprimesqrec & $95 < \qprimesqrec < 200 \GeVsq$ &  $105 < \qprimesqrec < 200 \GeVsq$ &
$105 < \qprimesqrec < 200 \GeVsq$ \\
\sph & $\sph > 0.4$ & $\sph > 0.4$ & $\sph > 0.5$ \\
\hline
$\epsilon_{ins}$ & $31.5$\% & $20.5$\% &$11.2$\% \\
%$\epsilon_{ins}/\epsilon_{dis}$ & 34-35 & 52-56 & 71-85 \\
$\epsilon_{dis}$ & 0.8-0.9 \% & 0.36-0.4 \% & 0.13-0.16\%\\
\end{tabular}
\end{center}
%\vspace{0.2cm}
\caption{Cut values, instanton (standard DIS) 
$\epsilon_{ins}$ ($\epsilon_{dis}$) efficiency 
in the three cut scenarios.}
\label{table:cuts}
\end{table}
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%


The numbers of events in the data and in the standard DIS Monte Carlo simulation
for the three cut scenarios are
summarised in table \ref{table:result}.
The quoted errors on the expected event numbers include the statistical and the
systematical uncertainties.
The experimental sources of the uncertainties
are: $4 \%$ on the absolute value of the hadronic energy scale
measured in the LAr calorimeter,
$1 \%$ on the electromagnetic energy scale,
$7 \%$  on the hadronic energy measured in the SpaCal
calorimeter, $3\%$ for the measurement of the
track momentum and $2$  {\rm mrad} for the polar
angle of the scattered positron. Moreover, an absolute
normalisation error of $1.5$\% for the accuracy of the luminosity
determination has been included. In the Monte Carlo the parton
density function have been reweighted to the ones measured
by H1. An overall error of $3 \%$ is assigned for the limited
precision of the proton structure function measurement.
%
The systematic error is dominated by the uncertainty in the
electromagnetic energy scale. 


%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
\begin{table}[t]
\begin{center}
\footnotesize
\begin{tabular}{|c|c|c|c|c|c|}
\hline
\multicolumn{2}{|c|} {\raisebox{0pt}[12pt][6pt]{(A) DATA: $3000$ }} &
\multicolumn{2}{|c|}{\raisebox{0pt}[12pt][6pt] {(B) DATA: $1332$} } &
\multicolumn{2}{|c|}{\raisebox{0pt}[12pt][6pt] {(C) DATA: $ 549$} }\\
\hline
\raisebox{0pt}[12pt][6pt] {CDM} & {MEPS}  &    
 {CDM} & {MEPS}  & 
 {CDM} & {MEPS}  \\ 
\hline
 \raisebox{0pt}[12pt][6pt] {$2469^{+242}_{-238}$} & {$2572^{+237}_{-222}$} &
  {$1005^{+82}_{-70}$} & {$1084^{+75}_{-46}$} &
  {$ 363^{+22}_{-26}$} & {$435^{+36}_{-22}$} \\
%\hline
%\raisebox{0pt}[12pt][6pt]{A} &{} &{}\\
%\\[22pt]
\hline
\end{tabular}
\end{center}
%\vspace{0.2cm}
\caption{Measured number of data events and expected standard DIS background
 for three cut scenarios. The errors are dominated by systematic uncertainties.}
\label{table:result}
\end{table}
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%


After the cuts of scenario $A$, $3000$ events are left in the data
while $2469 ^{+242} _{-238}$ ($2572 ^{+237} _{-222}$) are expected by the 
CDM (MEPS) Monte Carlo simulation. 
The distribution of the three cut observables is shown
in Fig.~\ref{fig:datamcinstmcA}. 
The excess in the data is mainly concentrated 
at low \nbx, at low \qprimesqrec values 
and is approximately equally large over the entire sphericity range. 

After the cuts of scenario $B$, $1332$ events are left in the data
while $1005^{+82}_{-70}$ ($1084^{+75}_{-46}$) are expected by the CDM 
(MEPS) Monte Carlo. 
The distribution of the three cut observables is shown
in Fig.~\ref{fig:datamcinstmcB}. 
The excess of the data over the standard DIS Monte Carlo is most pronounced
at low \nb and at low \qprimesqrec values. 

After the cuts of scenario $C$, $549$ events are left in the data
while $363^{+22}_{-26}$ ($435 ^{+36}_{-22}$) 
are expected by the CDM (MEPS) Monte Carlo. 
The distribution of the three cut observables is shown
in Fig.~\ref{fig:datamcinstmcC}.
The difference between data and standard DIS expectation
is most  pronounced at the lowest bin in \nb and for
$0.5 < \sph < 0.6$ and $100 < \qprimesqrec < 150$ \GeVsqx.

In all three cut scenarios more events are observed than
expected by the standard DIS Monte Carlo models.
The relatively large systematic experimental uncertainties ($5 - 10 \%$)
reduce the significance of the excess. 
However, they are not
able to explain the difference between data and standard DIS 
Monte Carlo simulation.
The two available standard DIS Monte Carlo
models based on leading order QCD matrix elements
and implementing different treatments of the higher
order parton emissions agree with each other within $20\%$.
They are both not able to explain the data.
With increasing separation of instanton induced
processes over normal DIS events an increasingly large
excess is seen in the data. 
A qualitative similarity between the difference between
data and DIS Monte Carlo simulation and the expected
shape of the I-signal is observed.
From a purely statistical point of
view the excess is significant, however the uncertainties
in the background estimation are largely unknown in this
extreme phase space region.
Whether this excess can be explained by instanton induced
processes or is simply due to an incomplete implementation
of higher order parton emissions or due to, for example, an incorrect
treatment of heavy quarks in the QCD Monte Carlo models
remains an open question.
%

The other three observables
which are sensitive discriminators for instantons from DIS events
are shown in Figs.~\ref{fig:datamcinstmcAother},
\ref{fig:datamcinstmcBother},\ref{fig:datamcinstmcCother}. 
%The excess in the data is not really compatible with the shape
%of the transverse energy of the particles in the instanton band 
%of the expected instanton signal.
The biggest discrepancy between data and standard 
DIS Monte Carlo simulation 
is found at the lowest transverse energy in the instanton band
where the expected contribution from I-processes is small.
For $\etb > 10$ \GeVx, where the instanton signal is expected to 
be largest, CDM predicts more events and MEPS
less events than found in the data. 
Only in the cut scenario with the highest sensitivity the data
slightly exceed both standard DIS expectations in this domain.
The difference between the two standard DIS Monte Carlo simulations
is not much smaller than the expected instanton signal. 
%In this phase space the data do not support an instanton contribution 
%as modelled in the implementation of the QCDINS Monte Carlo 
%cross section given by the QCDINS Monte Carlo. 
%
The shape of the \etb observable 
does therefore not particularly support the hypothesis that the observed
excess can be explained by I-processes as currently implemented in the
QCDINS Monte Carlo simulation.
The theoretical uncertainties on the default \xprime, \qprimesq 
parameters of QCDINS can, however, change the hadronic final state 
as discussed in \cite{inst:schremppdis00}.

%It should also been noted that the sharp cut on the minimal values
%of \xprime and \qprimesq implemented in the QCDINS program/used in this analysis
%is most probably not realised in nature in this simple manner.
%Due to the limited accuracy to reconstruct these quantities
%it is not possible to apply such requirements to the data.
%By comparison to lattice simulation, it has, however, been
%deduced that the \xprime and \qprimesq distributions are
%steeply decreasing towards lower values such that this should
%not significantly influence change the conclusions of this analysis. 

\subsection{Extraction of the Upper Limit}

The hadronic final state of instanton induced events
is strongly influenced by the energy 
$W_I^2 = \qprimesq (1-\xprime)/\xprime$ available for
the partons emerging from the instanton subprocess.
The final state topology does therefore
crucially depend on both the minimal cut values, where
instanton perturbation theory is expected to be valid,
and on the assumed \xprime and \qprimesq distributions
which are only under theoretical control for large 
\xprime and \qprimesqx. 

To minimize the theoretical input in the extraction of an
upper limit on the instanton production cross section,
small ranges of approximately constant \qprimesq and \xprime
are analysed. 
Events in a $5 \; \times \; 5$ grid
with  $0.2 \le \xprime \le 0.45$ (grid size $0.05$) and
with $60 \le \qprimesq \le 160$ \GeVsq (grid size $20$ \GeVsqx) 
have been simulated using QCDINS.
 
For each bin separately, events from one particular 
instanton type defined  by the chosen \xprime and \qprimesq values
are compared to all simulated standard DIS events.
The same strategy as described
in section \ref{sec:strategy} is applied to find the optimal
cuts to enhance the I-signal over the background
using the observables \nbx, \qprimesqrec and \sphx.
The combination ensuring an instanton efficiency
$\epsilon_{ins} > 10 \%$ and the maximal separation power
$\epsilon_{ins}/\epsilon_{dis}$ is chosen.
%
For each of the $25$ different resulting cuts the number of observed events
in the data and of the expected number
of standard DIS events is determined and an upper limit on
the instanton production cross section at $95\%$
confidence level (CL) is derived.
Two upper limits based on the two available  
standard DIS QCD simulations are extracted and the difference
between the two is treated as systematic uncertainty.
The result is shown in Fig.~\ref{fig:slim}
as a function of \xprime in bins of \qprimesq as hatched
area. Regions above the hatched area are excluded.

Given the known deficiencies of the standard DIS models 
to describe the hadronic final state in the HERA DIS regime,
it is, however, questionable whether the CDM and MEPS 
models are able to adequately describe the standard DIS 
background in this extreme corner of phase space where
(depending on the \xprimex,\qprimesq bin) only
$0.7 - 0.04 \%$ of the events in the total sample of DIS events
are expected to remain. 
These models were - before any cuts - only able to describe 
the observables used in this analysis to an accuracy of $20 \%$.
Moreover, after the cuts applied to enhance the expected instanton
signal large differences at low values of
the transverse energy in the band were found between the two models.
To be independent of the concrete modelling of the hadronic
final state of DIS events, an additional upper limit is extracted
where the expected standard DIS background is set to zero.
Whatever the ``true'' number of standard DIS events in
the selected corner of phase space is, the instanton signal
can certainly not be much bigger than the number of observed
events in the data. This upper limit on the instanton production
cross section is therefore the most conservative one,
since it only uses the expected topology of instanton events and
the number of events observed in the data. The limit is shown as 
a solid line in Fig.~\ref{fig:slim}. Regions above the curve
are excluded.

Instanton cross sections between $100$ and $1000$ \pb can be excluded. 
In Fig.~\ref{fig:slim} also the instanton cross section
evaluated in the Ringwald-Schrempp framework is indicated
in the region where I-perturbation theory is expected to be valid,
i.e. for large \xprime and \qprimesqx. 
The upper limits are above the predicted
cross sections in the fiducial region 
$\xprime > 0.35$ and $\qprimesq > 113$ \GeVsqx. 
However, these results can exclude
the continuation of the fast increase of the
instanton cross section towards lower values of \xprime
and \qprimesq as expected from a naive extrapolation
of I-perturbation theory into this domain.
This is the first experimental hint that the steep
rise of the I-cross section  
has to be attenuated in this domain.
This agrees with QCD calculations performed for zero flavours
on the lattice \cite{inst:rs-lat}.


\section{Conclusions}
We have searched for QCD instanton induced processes as
modelled in the Monte Carlo simulation program QCDINS
in deep-inelastic scattering in the kinematic range
$x >10^{-3}$, $0.1< y <0.6$ and $\theta_{el} >156^o$. 
We used three observables, the multiplicity in the instanton
band \nbx, the reconstructed quark virtuality entering the instanton
subprocess \qprimesqrec and the sphericity in the approximately reconstructed
instanton rest system \sphx, 
to select a QCD instanton enriched data sample.
Using a simple cut technique the standard DIS background can be
suppressed to the $0.1\%$ level, while $10 \%$ of the instanton induced
events are expected to be selected.
In this region $549$ events are observed and 
$363 ^{+22}_{-26}$ and $435 ^{+36}_{-22}$ 
are expected from the standard DIS background models
the colour dipol model and the matrix element and
parton shower model, respectively. 
With increasing sensitivity of instanton induced
processes over standard DIS events an increasingly large
excess is seen in the data. 
The shape of the excess in the observables \nbx, \sph and \qprimesqrec 
is qualitatively compatible with the expected instanton signal. 
However, the size of this
signal is at the level of discrepancies between the QCD models. 
The shapes of other observables (not used in the cuts)
are neither well reproduced by CDM nor by MEPS. Also 
the observed excess in the transverse energy in the instanton band 
is  not particularly favoured by the QCDINS
predictions. However, the QCDINS predictions can not be 
excluded given the uncertainties in the cross section
calculation and the modelling of the hadronic final state.

For various assumptions on the variables \xprime and
\qprimesq characterising the hard instanton processes
an upper limit on the instanton cross section is derived
which makes only use of the expected instanton hadronic
final state topology and the number of observed events in the data.
Instanton cross sections between $100$ and $1000$ \pb
can be excluded. This limit is larger than the 
predicted instanton cross section, but
excludes a steep rise as would be obtained from a naive extrapolation of 
I-perturbation theory. 
The absence of such steep rise is in accord
with lattice simulations for zero flavours. 


It should also be noted that the QCD Monte Carlo models 
have known deficiencies and fail to describe many aspects of
DIS data in the HERA regime.
%The estimation of the standard DIS background in the tails
%of distributions therefore has only a limited accuracy.
A better understanding of the formation of the hadronic
final state in DIS at the extreme end of the 
phase space relevant for instanton searches is required.
The expected background in the instanton
enriched sample is still large and in future more observables
and better discrimination techniques should be used to further
reduce the standard DIS background.


% **********************************************************************
% **********************************************************************
% **********************************************************************
\section{Acknowledgements}
% **********************************************************************
We thank A. Ringwald and F. Schrempp 
for many inspiring discussions and for their help.

We are grateful to the HERA machine group whose outstanding efforts
have made and continue to make this experiment possible.
We thank the engineers and technicians for their work in constructing and now 
maintaining the H1 detector, our funding agencies for financial support,
the DESY technical stuff for continual assistance, and the DESY directorate
for the hospitality which they extend to the non-DESY members of the
collaboration.


% **********************************************************************
% **********************************************************************
\bibliography{inst}

\newpage

% **********************************************************************

%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
\begin{figure}
\begin{center}
 \epsfig{figure=H1prelim-00-025.fig2.eps,
%bbllx=30,bblly=142,bburx=575,bbury=674,clip=,angle=0,
width=14.cm}
\end{center}
\caption{
Distribution of the number of charged particles in the instanton band,
of the sphericity in the rest system of all the final
state objects not associated to the 
current jet and of the reconstructed \qprimesqrecx. 
Shown are data and simulations of standard DIS events before cuts 
to enhance the instanton signal.
The predictions for the instanton induced process are too
small to be visible. 
The luminosity of the Monte Carlo simulation was scaled to the
luminosity of the data.
\label{fig:datamclin}}
\end{figure}
%
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
\begin{figure}
\begin{center}
 \epsfig{figure=H1prelim-00-025.fig3.eps,width=14.cm}
%bbllx=30,bblly=142,bburx=575,bbury=674,clip=,angle=0,width=14.cm}
\end{center}
\caption{As Fig.~\ref{fig:datamclin}, but with logarithmic scale.
As explained in the text, the instanton events have been generated
for $\qprimesq > 113$ \GeVsqx, as required theoretically. The apparent
penetration of I-events into the region of smaller $\qprimesq$ is due to the
limited accuracy of the \qprimesq reconstruction and  the experimental
resolution.
\label{fig:datamclog}}
\end{figure}
%
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
\begin{figure}
\begin{center}
 \epsfig{figure=H1prelim-00-025.fig4.eps,width=14.cm}
%bbllx=30,bblly=142,bburx=575,bbury=674,clip=,angle=0,width=14.cm}
\end{center}
\caption{Distribution of the total $E_t$ in the band,
of $(E_{in}-E_{out})/E_{in}$ and of the
transverse jet energy  in the inclusive DIS sample. 
The luminosity of the Monte Carlo was scaled to the
luminosity of the data.
\label{fig:datamclinother}}
\end{figure}
%
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
\begin{figure}
\begin{center}
 \epsfig{figure=H1prelim-00-025.fig5.eps,width=14.cm}
%bbllx=30,bblly=142,bburx=575,bbury=674,clip=,angle=0,width=14.cm}
\end{center}
\caption{Same as Fig. \ref{fig:datamclinother}, 
 but in logarithmic scale.
\label{fig:datamclogother}}
\end{figure}
%
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
\begin{figure}
\begin{center}
 \epsfig{figure=H1prelim-00-025.fig6.eps,
%bbllx=25,bblly=160,bburx=564,bbury=671,clip=,angle=0,
width=14.cm}
\end{center}
\caption{Shape normalised 
distribution of the number of charged particles in the instanton band,
of the sphericity in the rest system of all the final 
state objects not associated to the current jet 
and of the reconstructed \qprimesqrecx. Shown are 
standard DIS events and the instanton signal.
\label{fig:instmc}}
\end{figure}
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
\begin{figure}
\begin{center}
 \epsfig{figure=H1prelim-00-025.fig7.eps,width=14.cm}
%bbllx=30,bblly=142,bburx=575,bbury=674,clip=,angle=0,width=14.cm}
\end{center}
\caption{
Distribution of the number of charged particles in the instanton band, of
the sphericity in the rest system of all the final
state particles not associated to the current jet and of the reconstructed
\qprimesqrecx. Shown are data and the predictions for instanton induced
processes and standard DIS events after cuts  
to enhance the instanton signal.
The luminosity of the Monte Carlo simulation was scaled to the
luminosity of the data. 
The indicated cuts are called scenario A in the text.
\label{fig:datamcinstmcA}}
\end{figure}
%
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
\begin{figure}
\begin{center}
 \epsfig{figure=H1prelim-00-025.fig8.eps,width=14.cm}
%bbllx=30,bblly=142,bburx=575,bbury=674,clip=,angle=0,width=14.cm}
\end{center}
\caption{
Distribution of the number of charged particles in the instanton band,
of the sphericity in the rest system of all the final
state particles not associated to the 
current jet and of the reconstructed \qprimesqx. 
Shown are data and the predictions for instanton induced
processes and standard DIS events after cuts  
to enhance the instanton signal.
The luminosity of the Monte Carlo simulation was scaled to the
luminosity of the data. 
The indicated cuts are called scenario B in the text.
\label{fig:datamcinstmcB}}
\end{figure}
%
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
\begin{figure}
\begin{center}
 \epsfig{figure=H1prelim-00-025.fig9.eps,width=14.cm}
% bbllx=30,bblly=142,bburx=575,bbury=674,clip=,angle=0,width=14.cm}
\end{center}
\caption{
Distribution of the number of charged particles in the band,
of the sphericity in the rest system of all the final
state particles not associated to the 
current jet and of the reconstructed \qprimesq. 
Shown are data and the predictions for instanton induced
processes and standard DIS events after cuts  
to enhance the instanton signal.
The luminosity of the Monte Carlo simulation was scaled to the
luminosity of the data. 
The indicated cuts are called scenario C in the text.
\label{fig:datamcinstmcC}}
\end{figure}
%
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
\begin{figure}
\begin{center}
 \epsfig{figure=H1prelim-00-025.fig10.eps,width=14.cm}
%bbllx=25,bblly=160,bburx=564,bbury=671,clip=,angle=0,width=14.cm}
\end{center}
\caption{Distribution of the total $E_t$ in the instanton band', of
$(E_{in}-E_{out})/E_{in}$ and of  the
transverse jet energy after cuts to enhance the instanton
signal. 
The luminosity of the Monte Carlo simulation was scaled to the
luminosity of the data.
The indicated cuts are called scenario A in the text.
\label{fig:datamcinstmcAother}}
\end{figure}
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
%
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
\begin{figure}
\begin{center}
 \epsfig{figure=H1prelim-00-025.fig11.eps,width=14.cm}
%bbllx=25,bblly=160,bburx=564,bbury=671,clip=,angle=0,width=14.cm}
\end{center}
\caption{Distribution of the total $E_t$ in the band,
of $(E_{in}-E_{out})/E_{in}$ and of the
transverse jet energy  after cuts to enhance the instanton
signal. 
The luminosity of the Monte Carlo simulation was scaled to the
luminosity of the data. 
The indicated cuts are called scenario B in the text.
\label{fig:datamcinstmcBother}}
\end{figure}
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
%
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
\begin{figure}
\begin{center}
 \epsfig{figure=H1prelim-00-025.fig12.eps,width=14.cm}
% bbllx=25,bblly=160,bburx=564,bbury=671,clip=,angle=0,width=14.cm}
\end{center}
\caption{Distribution of the total $E_t$ in the band,
of $(E_{in}-E_{out})/E_{in}$ and of the
transverse jet energy in the band after cuts to enhance the instanton
signal. 
The luminosity of the Monte Carlo was scaled to the
luminosity of the data. 
The indicated cuts are called scenario C in the text.
\label{fig:datamcinstmcCother}}
\end{figure}
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
%
%
%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%%
\begin{figure}
\begin{center}
 \epsfig{figure=H1prelim-00-025.fig13.eps,width=14.cm}
\end{center}
\caption{Upper limit on the cross section for instanton induced
events as modelled by the QCDINS simulation as a function
of \xprime in bins of \qprimesq. 
Regions above the curves are excluded.
Also shown is the instanton cross section predicted in the
fiducial region $\xprime > 0.35$ and $\qprimesq > 113$ \GeVsqx. 
\label{fig:slim}}
\end{figure}
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\end{document}

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