The density of critical percolation clusters touching the boundaries of strips and
squares
Jacob J. H. Simmons∗ and Peter Kleban†
LASST and Department of Physics & Astronomy, University of Maine, Orono, ME 04469, USA
Kevin Dahlberg‡ and Robert M. Ziff§
MCTP and Department of Chemical Engineering,
University of Michigan, Ann Arbor, MI 48109-2136 USA
(Dated: November 10, 2018)
We consider the density of two-dimensional critical percolation clusters, constrained to touch one
or both boundaries, in infinite strips, half-infinite strips, and squares, as well as several related
quantities for the infinite strip. Our theoretical results follow from conformal field theory, and
are compared with high-precision numerical simulation. For example, we show that the density
of clusters touching both boundaries of an infinite strip of unit width (i.e. crossing clusters) is
proportional to (sin πy)−5/48{[cos(πy/2)]1/3 + [sin(πy/2)]1/3 − 1}. We also determine numerically
contours for the density of clusters crossing squares and long rectangles with open boundaries on
the sides, and compare with theory for the density along an edge.
Keywords: percolation, cluster density, crossing
I. INTRODUCTION
Percolation in two-dimensional systems is an area that has a long history, but remains under very active current
study. A number of very different methods has been applied to critical 2-D percolation, including conformal field
theory (CFT) [1], other field-theoretic methods [2], modular forms [3], computer simulation [4], Stochastic Loẅner
Evolution (SLE) processes [5] and other rigorous methods [6]. (Because the literature is so very extensive we have
cited only a few representative works.)
More specifically, there is a great deal of work of recent work studying universal properties of crossing problems
in critical percolation in two dimensions (i.e., [1, 3, 5, 7, 8, 9, 10, 11, 12]). Another interesting and also practically
important universal feature of percolation at the critical point is the density, defined as the number of times a
site belongs to clusters satisfying some specified boundary condition (such as clusters touching certain parts of the
boundary) divided by the total number of samples N , in the limit that N goes to infinity. This problem has been
addressed for clusters touching any part of the boundary of a system in various geometries, including rectangles, strips,
and disks, via conformal field theory [13] and by solving the problem for a Gaussian free field and then transforming
to other statistical mechanical models, including percolation [14]. In a recent Letter [30], we considered the problem
of clusters simultaneously touching one or two intervals on the boundary of a system, and considered cases where
those intervals shrink to points (anchor points). These results exhibit interesting factorization, are related to two-
dimensional electrostatics, and highlight the universality of percolation densities. Note that the density at a point
z of clusters which touch specified parts of the boundary is proportional to the probability of finding a cluster that
connects those parts of the boundary with a small region around the point z.
In this paper we consider the problem of the density ρb of critical percolation clusters in various geometries where
the clusters simultaneously touch both of the boundaries (i.e. crossing clusters), and several related quantities.
The first case we consider is an infinite strip, with boundaries parallel to the x-axis at y = 0 and y = 1, so the
crossing is in the vertical direction. (All our models are defined so that the crossing is vertical. Fig. 4 below illustrates
the geometries that we consider.) For the infinite strip we find (leaving out an arbitrary normalization constant here
and elsewhere) that
ρb(y) = (sinπy)
−5/48
. (1)
∗Electronic address: Jacob.Simmons@umit.maine.edu
†Electronic address: kleban@maine.edu
‡Electronic address: dahlberk@umich.edu
§Electronic address: rziff@umich.edu
http://arxiv.org/abs/0704.0901v2
mailto:Jacob.Simmons@umit.maine.edu
mailto:kleban@maine.edu
mailto:dahlberk@umich.edu
mailto:rziff@umich.edu
This may be compared to a previous result [13, 14] for clusters touching either the upper or lower boundary (or both)
which is simply given by
ρe(y) = (sinπy)
−5/48 . (2)
We also show that the density of clusters touching one boundary irrespective of touching the other is given by
ρ0(y) = (sinπy)
−5/48
ρ1(y) = (sinπy)
−5/48
, (4)
where ρ0 corresponds to those clusters touching the lower boundary at y = 0, and ρ1 corresponds to those clusters
touching the upper boundary at y = 1. (Note that ρ0 is the analog of the order parameter profile 〈σ〉+,f for the Ising
case (see Eq. (16) in [19].) We also find expressions for clusters touching one boundary and not the other, which are
combinations of the above results.
Perhaps the main new theoretical result in the above is (3) (or equivalently (4)), which follows straightforwardly
from the results in [30]. The derivation is given in section II.
A second type of theoretical prediction gives the density variation along a boundary (the general expressions is in
(15)). This is used to predict the density along the edge in several geometries (see (17), (18), and (19) below).
The above theoretical results are found to be consistent with numerical simulations to a high degree of accuracy.
We include the results of numerical simulations of the density contours of clusters crossing square and rectangular
systems vertically, with open boundaries on the sides, and compare with theory along the boundaries.
Our theoretical treatment is related to previous use of conformal field theory to study order parameter profiles in
various 2-D critical models with edges and similar research [13, 15, 16, 17, 18, 19, 20, 21, 22, 23, 24, 25, 26, 27, 28].
(Note that the density which we consider is the expectation value of the spin operator in percolation, which is the
order parameter in this setting.) Many of these prior results make use of the original Fisher-de Gennes proposal [29]
for the behavior of the order parameter at criticality near a straight edge. In this paper, we limit ourselves to critical
percolation. We also include the results of high-precision computer simulations. In addition, the formula (15) for the
density along the edge of a system is new, to our knowledge.
Note that, because of the fractal nature of critical percolation clusters, the density of clusters is, strictly speaking,
zero everywhere in the system. However, if we properly renormalize the density as the lattice mesh size goes to zero,
the density can remain finite. At the boundaries, for some quantities, this results in the density diverging, as for
ρe(y) at y = 0 and y = L (but remaining integrable). For ρb(y) of equation (1), on the other hand, the renormalized
density remains finite everywhere. When comparing to numerical simulations, one has to normalize the data so
that the densities coincide with the theoretical prediction using whatever normalization convention is chosen for the
theoretical results. The resulting normalization constant, which must be applied to the numerical data, is specific for
each system and is non-universal.
In the following sections, we first give the theoretical derivation of our infinite strip formulas above. Then we
present the numerical results. This is followed by numerical results on square and (long) rectangular systems. These
are compared with theory for the density along the edges of these systems. We end with a few concluding remarks.
II. THEORY FOR THE INFINITE STRIP
We first consider the density of critical percolation clusters which span the sides of an infinite 2-D strip. We can
find the density predicted by conformal field theory [31] using the results of [30]. In that article we showed that in
the upper half plane the density ρ of clusters connected to an interval (xa, xb) is
ρ(z, xa, xb) ∝ (z − z̄)−5/48F
(xb − xa)(z̄ − z)
(z̄ − xa)(xb − z)
, (5)
where the function F (η) was determined by conformal field theory and takes on one of two forms,
F±(η) =
. (6)
If we parameterize z as z = reiθ and let xa → 0 and xb → ∞, then η = 1− e2iθ and using (6) we can rewrite (5) as
ρ+(r, θ, xa → 0, xb → ∞) ∝ (r sin θ)−5/48[cos(θ/2)]1/3 (7)
ρ−(r, θ, xa → 0, xb → ∞) ∝ (r sin θ)−5/48[sin(θ/2)]1/3 . (8)
For the positive real axis θ → 0 and ρ+ ∼ θ−5/48 while for the negative real axis θ → π and ρ+ ∼ (π− θ)11/48. The
powers here arise from the fixed and free boundary exponents, respectively, in the bulk-boundary operator product
expansion of the magnetization operator ψ [30]. (More specifically, as it approaches the boundary, ψ ∼ 1 or ψ ∼ φ1,3,
which have conformal dimensions 0 and 1/3, respectively.) This shows that ρ+ is the density of clusters attached to
the positive axis. Because ρ−(r, θ) = ρ+(r, π− θ), it follows that ρ− is the density of clusters attached to the negative
real axis.
The final density that we need is that of clusters connected arbitrarily to the axis. This is given by 〈ψ(z, z̄)〉fixed ∝
(z − z̄)−5/48 [13, 14, 30] which may also be written
ρa(r, θ) ∝ (r sin θ)−5/48 . (9)
These densities are unnormalized. However for points that are short distances above the positive (negative) axis,
but very far from the origin, the relation ρ+(−) ≈ ρa holds. This condition holds since the points are far from the free
boundary, and thus dominated by the fixed boundary. It is satisfied by our expressions for ρ+, ρ−, and ρa, so they
are properly normalized relative to one another.
We next map these densities into the infinite strip w ∈{x+ iy| x ∈ (−∞,∞), y ∈ (0, 1)} using
w(z) =
log(z) . (10)
This leads to the expressions for ρ0(y), ρ1(y), and ρe(y) given by equations (3), (4), and (2), respectively.
Using these functions we can also determine the densities of clusters that touch one side but not the other,
ρ01̄(y) = ρe(y)− ρ1(y) = (sinπy)−5/48
1− [cos(πy/2)]1/3
ρ10̄(y) = ρe(y)− ρ0(y) = (sinπy)−5/48
1− [sin(πy/2)]1/3
. (12)
In a similar manner we can find the density of clusters touching both sides, ρb(y). Adding ρ0 and ρ1 includes all
configurations that touch either side, but double counts the clusters that touch both sides. Subtracting ρe leaves only
those clusters that touch both sides of the strip. Thus
ρb(y) = ρ0(y) + ρ1(y)− ρe(y) , (13)
which gives equation (1).
III. SIMULATIONS FOR THE INFINITE STRIP
To approximate the infinite strip, we considered rectangular systems with periodic boundary conditions in the
horizontal direction, for both site and bond percolation on square lattices. Here we report our results for site
percolation on the square lattice, for a system of 511 (vertical) × 2048 (horizontal) sites, at p = pc = 0.5927462
[32]. We generated 500,000 samples to compute the average densities, using a Leath-type of algorithm to find all
clusters touching the upper and lower boundaries.
The aspect ratio of the rectangle used in our simulations was 2048/511 = 4.008 . . ., which might seem a bit small.
However, since the correlation length of the system is governed by the width of the rectangle (511), the effect of the
finite ratio drops off exponentially with the length of the rectangle, so our results should be very close to those of
an infinite strip, an expectation which is born out by the results described below. (Furthermore, the probability of
finding a horizontally wrapping cluster drops exponentially with the aspect ratio, so if a longer rectangle were used,
very few wrapping clusters would be found and the data would have poor statistics.)
The agreement of predicted and simulated values is excellent. In Fig. 1 we show the results for ρb(y) with no
adjustments, other than an overall normalization (in particular, the extrapolation length a, described below, is set to
zero). Fig. 2 (upper set of points) shows the ratio of simulation to theoretical results, equation (13). Most points fall
within 1%, except those right near the boundary. However, we can do better.
When comparing simulations on a (necessarily) finite lattice with the results of a continuum theory, there is the
question, due to finite-size and edge effects, of what value of the continuous variable y should correspond to the lattice
variable Y — specifically, where the boundary of the system should be placed. On the lattice, the density goes to zero
at Y = 0 and Y = 512. A näıve assignment of the continuum coordinate would therefore be y = Y/512. However,
we can get a better fit to the data near the boundaries by assuming that the effective boundary is a distance a (in
units of the lattice spacing) beyond the lattice boundaries — that is, at Y = −a and Y = 512 + a. The distance a is
0 0.2 0.4 0.6 0.8 1
FIG. 1: (Color online).
ρb(y) vs. y. Open violet circles, theoretical values from equation (13) (here normalized to 1 at the center point), using (14)
with a = 0. Blue dots: results from simulations.
an effective “extrapolation length” where the continuum density far from the wall extrapolates to the value zero [33].
This is accomplished by defining the continuum variable y by
y = (Y + a)/(512 + 2a) . (14)
Then, Y = −a corresponds to y = 0 and Y = 512 + a corresponds to y = 1. Note, Y = 0 corresponds to
y = a/(512 + 2a) and Y = 512 corresponds to y = (512 + a)/(512 + 2a) = 1 − a/(512 + 2a), and so the theoretical
extrapolated density ρb(y) will be greater than zero at these points on the actual boundary. The spacing between all
points is stretched by a small amount because of the denominator in equation (14), but this stretching does not have
much effect on the behavior of ρb near the center. The main effect of a on the shape of the theoretical curves of ρb is
near the boundaries.
By choosing an extrapolation length of a = 0.26, we can get a much better fit of the data, as can be seen in Fig. 2
(lower set of points). A plot of the data analogous to Fig. 1 puts most of the data points right in the center of the
theoretical circles, but would barely be visible when plotted on this scale. With a = 0.26, the error is now reduced to
less than 0.1%, except right near the boundaries, as can be seen in Fig. 2. A more thorough study of the extrapolation
coefficient a would require the study of different sized lattices, and the demonstration that a is independent of the
lattice size. We have not carried this out. Note, however, that a constant a implies that if one keeps the physical size
of the lattice fixed (so that the increasing number of lattice points makes the mesh size go to zero), the extrapolation
length, measured in physical units, will also go to zero.
Note also that the distance in the y directions was 511 rather than 512 because we used one row at Y = 0, in
conjunction with the periodic boundary conditions, to represent both horizontal boundaries of the system on the
lattice. That is, Y = 1 and Y = 511 are the lowest and highest rows where we occupy sites in the system, where Y
represents the lattice coordinate in the vertical direction.
We note that these simulations were carried out before the theoretical predictions were made.
We have also carried out simulations measuring the density of clusters touching one edge, ρ0(y). The results are
shown in Fig. 3. We also plot the results of the theoretical prediction, equation (3), on the same plot, and find
agreement within 0.5% without using an extrapolation length a.
0.995
1.005
1.015
1.025
1.035
0 0.1 0.2 0.3 0.4 0.5 0.6 0.7 0.8 0.9 1
FIG. 2: (Color online). Ratio of simulation to theoretical results for ρb(y) with a = 0 (upper set of points) and a = 0.26 (lower
set of points)
0 0.2 0.4 0.6 0.8 1
FIG. 3: (Color online). Density of clusters touching lower boundary, ρ0(y), as a function of y, both simulation (dots) and
theory (open circles), equation (3).
(c) (d)
FIG. 4: Sketches of the cases considered. Solid (dashed) boundary lines represent fixed (open) boundary conditions. Curved
lines indicate crossing clusters; the density ρb is evaluated along the lines with arrowheads. (a) is the infinite strip, cf. e.g.
equation (1); (b) the square (Fig. 6), (c) and (d) vertical half-infinite strips ((17) and (18), respectively); (e) horizontal
half-infinite strip (19).
IV. PERCOLATION ON A SQUARE AND SEMI-INFINITE STRIP
In this section, we consider the density of crossing clusters on a square with open boundaries and also on a (long)
rectangle. We compare the numerical results with the predictions of conformal field theory for the density along an
edge. The various cases considered are illustrated in Fig. 4.
Note that, as mentioned, the crossing is always in the vertical direction. In a slight abuse of notation, we use ρb for
the density of a clusters that touch both anchoring intervals in all cases. The different situations may be distinguished
by the arguments of ρb, e.g. ρb(y) for the infinite strip, where there is no x dependence, and ρb(x, y = 0) along the
bottom of the semi-infinite strip as in (17) below.
Our simulations of percolation densities on an open square examined clusters that cross in the vertical direction,
0 100 200 300 400 500
FIG. 5: (Color online) Contours of constant densities 0.625, 0.75, 0.875, 15/16=0.9375, 31/32=0.96875, 63/64 = 0.984375,
127/128 = 0.9921875, and 1 (outside to center) of clusters touching both the top and bottom edges, with open b.c. on the sides,
for a system of 511× 511 sites.
with open boundary conditions on the left- and right-hand sides. We considered site percolation on a square lattice
of 511× 511, with 2,000,000 samples generated. The resulting contours are shown in Fig. 5. As in the periodic case,
the density goes to zero at the upper and lower boundaries because, compared to an infinite system, these boundaries
intersect many possible crossing paths, leading to large holes in the clusters near the boundaries. As a consequence,
relatively few points on the boundary will be part of the crossing clusters, and in the limit that the mesh size goes to
zero, their density evidently goes to zero. The density also goes to zero on the sides because of the open conditions
there. Interestingly, the contour curves are almost symmetric in the horizontal and vertical directions, indicating that
the anchoring and open boundaries have a similar effect on the density.
We have not carried out a field-theory calculation to find the density inside the square or rectangular systems. To
do so requires a six-point function whose calculation would be unwieldy.
It is however relatively easy to calculate the variation of the density along the bottom edge of the square, now
normalized so that the density remains non-zero as the mesh size goes to zero. To do this, we consider the density of
crossings from one of the anchoring intervals to a single point on the other interval, using the boundary spin operator.
Now crossing from the top edge to one point x on the bottom edge (which is given by a three-point function, depending
only on x and λ) automatically implies crossing from the top to bottom (which is given by a four-point function,
depending only on λ). Therefore the density at x is proportional to the ratio of the former to the latter. It follows
generally that, up to a (λ-dependent) multiplicative constant, one has [34]
ρ(x) =
|z′(x)|
1− λz(x)
. (15)
Here z(w) maps the region of interest (w) onto the 1/2-plane (z), x is the w-coordinate along the anchoring interval
of interest, and λ is the conformally invariant cross-ratio for the anchoring points. For a rectangle, this depends on
the aspect ratio r = K(
1− λ)/K(
λ) [1, 35].
The mapping for the square is
z(w) = 1− ℘
(iw + 1)K(2); 4, 0
, (16)
with ℘(u; g2, g3) the Weierstrass elliptic function and K(z) the elliptic integral function. This mapping takes a unit
square x, y ∈ (0, 1) into the upper half plane. For the square λ = 1/2, and we can take x ∈ (0, 1). In Fig. 6 we
compare the measurement and theory. Clearly the agreement is excellent.
In the case of a half-infinite strip x ∈ (0, 1), y ∈ (0,∞), the density of sites along the x-axis belonging to clusters
crossing vertically is found from (15) using z(w) = sin2(πw/2), and λ = 0. This gives
ρb(x, y = 0) = (sinπx)
1/3 . (17)
Of course, for an infinite strip, the probability of crossing (in the long direction) is zero, so one must consider the
limit of a large system, and calculate the density given that crossing takes place, and take the limit that the length of
the rectangle goes to infinity. It turns out that numerically, the density at the edge for the square, equations (15,16),
differs only very slightly from that of the half-infinite strip, given by equation (17). From the point of view of the
density along an anchoring edge, the square is not much different from the half-infinite strip.
For y ≫ 0 in the above half-infinite strip (or equivalently for any y for a fully infinite strip in the vertical direction)
one can also find the density along the x-direction of the vertically crossing clusters in closed form
ρb(x, y ≫ 0) = (sin πx)11/48 . (18)
This function may be found by transforming the density of clusters connecting two boundary points, derived in [30],
into the infinite strip. We then take the limit as the two anchoring points move infinitely far away in opposite
directions, while normalizing the density so that it remains finite. (Related order-parameter profiles for the Ising
case are studied in [22].) Interestingly, a plot of this density profile (written as a function of y rather than x) is
very similar in appearance to that of the vertically crossing clusters ρb(y) given in equation (1) and plotted in Fig. 1.
When normalized so that they have the same value at y = 1/2, the maximum difference between the two is at y = 0
and y = 1, where (18) is only 1.5 % below (1). This small difference indicates that open boundaries and anchoring
boundaries have similar effects on the density of the crossing percolation clusters, and is consistent with the near
symmetry seen in the contours in Fig. 5.
We can also find the density along the left and right (open) edges. For the case of a half-infinite strip rotated by
90◦ with respect to the one above, (y ∈ (0, 1), x ∈ (0,∞)), we find
ρb(x = 0, y) = (sinπy)
, (19)
which is similar in form to ρb(y) of equation (1) (which in fact corresponds to x≫ 0 for the geometry considered here)
but with different exponents. This similarity arises because the derivations of (19) and (13) are virtually identical,
except that for (19) we leave a free interval between the two anchoring intervals (where the boundary spin operator
sits) which is mapped to the end of the half-infinite strip using sine functions. Comparison with numerical data
(not shown) for the density at the short edge of a rectangle of aspect ratio 8 to approximate the infinite strip shows
excellent agreement with (19).
V. FURTHER COMMENTS AND CONCLUSIONS
If we consider densities raised to the sixth power (compare Ref. [30]), we find a Pythagorean-like relation involving
ρe(y)
3, ρ0(y)
3, and ρ1(y)
3 (which we present without interpretation),
ρ0(y)
6 + ρ1(y)
6 = ρe(y)
6 . (20)
There seems to be no simple relation involving ρb(y) other than its basic definition given in equation (13). For the
corresponding quantities at the edge of the strip as in (19), the power in equation (20) is 3 rather than 6.
Although the overall normalization of a density such as ρb(y) (for the infinite strip, see (1)) is arbitrary, we can fix
its value by requiring that
ρb(y)dy = 1 . (21)
That is, we define ρb(y) = B sin(πy)
−5/48(cos(πy/2)1/3+sin(πy/2)1/3−1) where B is a constant. Then equation (21)
yields
= 1.46408902 . . . . (23)
0 0.2 0.4 0.6 0.8 1
Theory
Simulation
FIG. 6: (Color online) Density of vertically crossing clusters ρb(x, 0) along the lower boundary, in a square system with open
boundaries on the horizontal sides. Red line: theory, equation (15), black dots: simulation results.
Another choice of B is to make ρb(1/2) = 1, which yields B = (2
5/6 − 1)−1 = 1.27910371 . . .
In many problems of percolation density profiles, the density goes to infinity at a boundary point, such as occurs for
ρ0(y) when y → 0. Interestingly, in the case considered here of clusters touching both boundaries, ρb(y), the density
goes to zero at those boundaries and remains finite everywhere.
To highlight the difference between densities of all clusters touching a boundary vs. the densities of crossing clusters
touching one boundary, we consider the limit that the strip width becomes infinite, so that the system becomes a
half-plane. Because we have written our results for a strip of fixed (unit) width, this density is given by the behavior
of ρ for small y. The density of all clusters touching the x-axis is thus found from equation (3) (or [13, 14]) to be
ρ0 ∼ y−5/48 , (24)
where we have left off the coefficient because the normalization is arbitrary. This density diverges at y = 0 because
it is much more likely to find sites belonging to these clusters near the x-axis. On the other hand, the density of
crossing clusters touching the x-axis is found from equation (1) in the limit y → 0,
ρb ∼ y11/48 . (25)
In this case, the density increases as y increases, in contrast to (24), and goes to zero at the anchoring boundary, for
the reason mentioned above.
Behavior identical to (25) also follows from the small-x expansion of ρb(x, y ≫ 0) given by (18), which represents
the behavior of the density of the vertically spanning clusters at the open boundary. Thus, near the boundaries (but
away from the corners), the open and anchoring boundary conditions have identical effects on the density of the
crossing clusters.
In conclusion, we have studied the density of vertically percolating clusters in a square system, as well as for half-
infinite and infinite strips extending in either the horizontal or vertical direction. The various cases considered are
illustrated in Fig. 4.
For the infinite strip, Fig. 4(a), the density for crossing clusters is given by (19) and compared with numerical
simulations in Figs. 1 and 2. For the square, Fig. 4(b), we find theoretical results for the anchoring edge densities
(see (15) and (16) and Fig. 6), as well as numerical results for the density in the interior (Fig. 5), which exhibit an
interesting near symmetry. For the half-infinite strip in the horizontal direction, Fig. 4(e), the density ρb(x = 0, y) at
the left open boundary is given by (19), and at x ≫ 0 (or equivalently, for an infinite strip), the density is given by
(1). For a half-infinite strip in the vertical direction, the density along the lower anchoring boundary (Fig. 4(c)) is
given by (17) while for y ≫ 0 (Fig. 4(d)) the density is given by (18). For the half-infinite systems, the densities near
a wall are given by the same power-law (25) regardless of whether it anchors the crossing clusters or is open. Note
that all of our theoretical predictions were confirmed by computer simulation.
For the future, it would be interesting to study analogous properties for Fortuin-Kasteleyn (FK) clusters of the
critical Ising and Potts models.
VI. ACKNOWLEDGMENTS
This work was supported in part by the National Science Foundation under grants numbers DMS-0553487 (RMZ)
and DMR-0536927 (PK).
[1] J. L. Cardy, Critical percolation in finite geometries, J. Phys. A 25 L201-206 (1992) [arXiv: hep-th/9111026].
[2] B. Duplantier, Higher conformal multifractality, J. Stat. Phys. 110 691-738 (2003) [arXiv: cond-mat/0207743]; Conformal
fractal geometry and boundary quantum gravity, preprint [arXiv: math-ph/0303034].
[3] P. Kleban and Don Zagier, Crossing probabilities and modular forms, J. Stat. Phys. 113 431-454 (2003) [arXiv: math-
ph/0209023].
[4] P. Kleban and R. M. Ziff, Exact results at the two-dimensional percolation point, Phys. Rev. B 57 R8075-R8078 (1998)
[arXiv: cond-mat/9709285].
[5] J. Dubédat, Excursion decompositions for SLE and Watts’ crossing formula, Probab. Theory Related Fields, no. 3, 453-488
(2006) [arXiv: math.PR/0405074].
[6] M. Aizenman, Scaling Limit for the Incipient Spanning Clusters, in Mathematics of Multiscale Materials; the IMA Volumes
in Mathematics and its Applications (K. Golden, G. Grimmett, R. James, G. Milton, and P. Sen, eds.), Springer (1998)
[arXiv: cond-mat/9611040].
[7] R. P. Langlands, C. Pichet, Ph. Pouliot and Y. Saint-Aubin, On the universality of crossing probabilities in two-dimensional
percolation, J. Stat. Phys. 67 553-574 (1992).
[8] S. Smirnov, Critical percolation in the plane, C. R. Acad. Sci. Paris Sr. I Math. 333 no. 3, 239-244 (2001).
[9] Bertrand Berche, Jean-Marc Debierre and Hans-Peter Eckle, Surface shape and local critical behavior: The percolation
problem in two dimensions, Phys. Rev. E 50 4542-4550 (1994).
[10] G. M. T. Watts, A crossing probability for critical percolation in two dimensions, J. Phys. A 29 L363-L368 (1996) [arXiv:
cond-mat/9603167].
[11] Robert M. Ziff, Spanning probability in 2D percolation, Phys. Rev. Lett. 69 2670-2673 (1992).
[12] Oleg A. Vasilyev, Universality of the crossing probability for the Potts model for q = 1, 2, 3, 4, Phys. Rev. E 68 026125
(2003).
[13] Theodore W. Burkhardt and Erich Eisenriegler, Universal order-parameter profiles in confined critical systems with bound-
ary fields, J. Phys. A: Math. Gen. 18 L83-L88 (1985).
[14] Ivica Reš and Joseph P. Straley, Order parameter for two-dimensional critical systems with boundaries, Phys. Rev. B 61,
14425-14433 (2000) [arXiv: cond-mat/9910467].
[15] T. W. Burkhardt and J. L. Cardy Surface critical behaviour and local operators with boundary-induced critical profiles, J.
Phys. A: Math. Gen. 20 L233-L238 (1987).
[16] T. W. Burkhardt and I. Guim Bulk, surface, and interface properties of the Ising model and conformal invariance, Phys.
Rev. B 36 2080-2083 (1987).
[17] J. L. Cardy, in Phase transitions and critical phenomena, C. Domb and J. L. Lebowitz, Vol. 11, Academic, New York
(1987).
[18] J. L. Cardy Universal critical-point amplitudes in parallel-plate geometries, Phys. Rev. Lett. 65 1443-1445 (1990).
[19] T. W. Burkhardt and T. Xue Density profiles in confined critical systems and conformal invariance, Phys. Rev. Lett. 66
895-898 (1991).
[20] T. W. Burkhardt and T. Xue Conformal invariance and critical systems with mixed boundary conditions, Nucl. Phys. B
354 653-665 (1991).
[21] T. W. Burkhardt and E. Eisenriegler Conformal theory of the two-dimensional 0(N) model with ordinary, extraordinary,
and special boundary conditions, Nucl. Phys. B 424 487-504 (1994).
[22] Löıc Turban and Ferenc Iglói, Off-diagonal density profiles and conformal invariance, J. Phys. A: Math. Gen. 30 L105-L111
(1997) [arXiv:cond-mat/9612128].
[23] Ferenc Iglói and Heiko Rieger Density Profiles in Random Quantum Spin Chains, Phys. Rev. Lett. 78 2473-2476 (1997)
[arXiv:cond-mat/9609263].
[24] E. Carlon and F. Iglói Density profiles, Casimir amplitudes, and critical exponents in the two-dimensional Potts model: A
density-matrix renormalization study, Phys. Rev. B 57 7877-7886 (1998) [arXiv:cond-mat/9710144].
[25] D. Karevski, L. Turban and F. Iglói Conformal profiles in the Hilhorst-van Leeuwen model, J. Phys. A: Math. Gen. 33
2663-2673 (2000) [arXiv:cond-mat/0003310].
[26] U. Bilstein The XX-model with boundaries: III. Magnetization profiles and boundary bound states, J. Phys. A: Math. Gen.
33 7661-7686 (2000) [arXiv:cond-mat/0004484].
[27] M. Krech Surface scaling behavior of isotropic Heisenberg systems: Critical exponents, structure factor, and profiles, Phys.
Rev. B 62 6360-6371 (2000) [arXiv:cond-mat/0006448].
[28] L. Turban Conformal off-diagonal boundary density profiles on a semi-infinite strip, J. Phys. A: Math. Gen. 34 L519L523
(2001) [arXiv:cond-mat/0107235].
[29] M. E. Fisher and P. G. de Gennes, Phénomènes aux parois dans un mélange binaire critique: physique des collöıdes , C.
R. Acad. Sci., Paris B 287 207 (1978).
[30] Peter Kleban, Jacob J. H. Simmons, and Robert M. Ziff, Anchored critical percolation clusters and 2D electrostatics, Phys.
Rev. Lett. 97 115702 (2006) [arXiv: cond-mat/0605120].
[31] A. A. Belavin, A. M. Polyakov, and A. B. Zamolodchikov, Infinite conformal symmetry in two-dimensional quantum field
theory, Nucl. Phys. B241, 333-380 (1984).
[32] M. E. J. Newman and R. M. Ziff, Efficient Monte Carlo algorithm and high-precision results for percolation, Phys. Rev.
Lett. 85 4104-4107 (2000) [arXiv: cond-mat/0005264].
[33] R. M. Ziff, Effective boundary extrapolation length to account for finite-size effects in the percolation crossing function,
Phys. Rev. E 54 2547-2554 (1996).
[34] Peter Kleban, Jacob J. H. Simmons, and Robert M. Ziff, Crossing, connection and cluster density in critical percolation
on trapezoids, Preprint (2007).
[35] R. M. Ziff, On Cardy’s formula for the critical crossing probability in 2d percolation, J. Phys. A: Math. Gen. 28, 1249-1255
(1995).
	Introduction
	Theory for the infinite strip
	Simulations for the infinite strip
	Percolation on a square and semi-infinite strip
	Further comments and conclusions
	Acknowledgments
	References

  We consider the density of two-dimensional critical percolation clusters,
constrained to touch one or both boundaries, in infinite strips, half-infinite
strips, and squares, as well as several related quantities for the infinite
strip. Our theoretical results follow from conformal field theory, and are
compared with high-precision numerical simulation. For example, we show that
the density of clusters touching both boundaries of an infinite strip of unit
width (i.e. crossing clusters) is proportional to $(\sin \pi
y)^{-5/48}\{[\cos(\pi y/2)]^{1/3} +[\sin (\pi y/2)]^{1/3}-1\}$.
  We also determine numerically contours for the density of clusters crossing
squares and long rectangles with open boundaries on the sides, and compare with
theory for the density along an edge.

Introduction
	Theory for the infinite strip
	Simulations for the infinite strip
	Percolation on a square and semi-infinite strip
	Further comments and conclusions
	Acknowledgments
	References
